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OSMANIA UNIVERSITY LIBRARY 

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MECHANICS 



THE MACMILLAN COMPANY 

NEW YORK BOSTON CHICAGO DALLAS 
ATLANTA SAN FRANCISCO 

MACMILLAN & CO., LIMITED 

LONDON BOMBAY CALCUTTA 
MELBOURNE 

THE MACMILLAN COMPANY 
OF CANADA, LIMITED 

TORONTO 



MECHANICS 



BY 
WILLIAM FOGG OSGOOD, PH.D., LL.D. 

PERKINS^ PROFESSOR OF MATHEMATICS, EMERITUS 
IN HARVARD UNIVERSITY 



NEW YORK 
THE MACMILLAN COMPANY 

1949 



COPYRIGHT, 1937, 
BY THE MACMILLAN COMPANY. 



All rights reserved no part of this book may be 
reproduced in any form without permission in writing 
from the publisher, except by a reviewer who wishes 
to quote brief passages in connection with a review 
written for inclusion in magazine or newspaper. 

Published June, 1937. 

Reprints! Nov. 1946. 

Reprinted, May, 1948. 

Reprinted November, 1949 



ST UP AND ELECTROTYPED BY J. S. GUSHING CO. 
PRINTED IN THE UNITED STATES OF AMERICA 



PREFACE 

Mechanics is a natural science, and like any natural science 
requires for its comprehension the observation and knowledge of a 
vast fund of individual cases. Arid so the solution of problems is 
of prime importance throughout all the study of this subject. 

But Mechanics is not an empirical subject in the sense in which 
physics and chemistry, when dealing with the border region of tUe 
human knowledge of the day are empirical. The latter take 
cognizance of a great number of isolated facts, which it is not as 
yet possible to arrange under a few laws, or postulates. The laws 
of Mechanics, like the laws of Geometry, so far as first approxima- 
tions go the laws that explain the motion of the golf ball or the 
gyroscope or the skidding automobile, and which make possible 
the calculation of lunar tables and the prediction of eclipses 
these laws are known, and will bo as new arid important two 
thousand years hence, as in the recent past of science when first 
they emerged into the light of day. 

Here, then, is the problem of training the student in Mechanics 
to provide him with a vast fund of case material and to develop 
in him the habits of thought which refer a new problem back to the 
few fundamental laws of the subject. The physicist is keenly 
alive to the first requirement and tries to meet it both by simple 
laboratory experiments and by problems in the part of a general 
course on physics which is especially devoted to "Mechanics." 
The interest of the mathematician too often begins with virtual 
velocities and d'Alembert's Principle, and the variational principles, 
of which Hamilton's Principle is the most important. Both arc 
right, in the sense that they are dping nothing that is wrong ; but 
each takes such a fragmentary view of the whole subject, that his 
work is ineffectual. 

The world in which the boy and girl have lived is the true 
laboratory of elementary mechanics. The tennis ball, the golf 
ball, the shell on the river ; the automobile good old Model T, 
in its day, and the home-made autos and motor boats which 



vi PREFACE 

youngsters construct and will continue to construct the amateur 
printing press ; the games in which the mechanics of the body is a 
part ; all these things go to provide the student with rich laboratory 
experience before he begins a systematic study of mechanics. It 
is this experience on which the teacher of Mechanics can draw, and 
draw, and draw again. 

The Cambridge Tripos of fifty years and more ago has been 
discredited in recent years, and the criticism was not without 
foundation. It was a method which turned out problem solvers 
so said its opponents. But it turned out a Clerk Maxwell and it 
vitally influenced the training of the whole group of English 
physicists, whose work became so illustrious. In his interesting 
autobiography, From Emigrant to Inventor, Pupin acknowledges in 
no uncertain terms the debt he owes to just this training, and to 
Arthur Gordon Webster, through whom he first came to know 
this method a method which Benjamin Osgood Peirce also 
prized highly in his work as a physicist. And so we make no 
apologies for availing ourselves to the fullest extent of that which 
the old Tripos Papers contributed to training in Mechanics. But 
we do not stop there. After all, it is the laws of Mechanics, their 
comprehension, their passing over into the flesh and blood of our 
scientific thought, and the mathematical technique and theory, 
that is our ultimate goal. To attain to this goal the mathematical 
theory, absurdly simple as it is at the start, must be systematically 
inculcated into the student from the beginning. In this respect 
the physicists fail us. Because the mathematics is simple, they 
do not think it important to insist on it. Any way to get an 
answer is good enough for them. But a day of reckoning comes. 
The physicist of to-day is in desperate need of mathematics, and 
at best all he can do is to grope, trying one mathematical expedient 
after another and holding to no one of these long enough to test 
it mathematically. Nor is he to be blamed. It is the old (and 
most useful) method of trial and error he is employing, and must 
continue to employ for the present. 

Is the writer on Mechanics, per contra, to accept the challenge 
of preparing the physicist to solve these problems? That is too 
large a task. Rather, it is the wisdom of Pasteur who said : 
"Fortune favors the prepared mind" that may well be a guide for 
us now and in the future. What can be done, and what we havo 
attempted in the present work, is to unite a broad and deep knowv 



PREFACE vii 

edge of the most elementary physical phenomena in the field of 
Mechanics with the best mathematical methods of the present 
day, treating with completeness, clarity, and rigor the beginnings 
of the subject ; in scope not restricted, in detail not involved, in 
spirit scientific. 

The book is adapted to the needs of a first course in Mechanics, 
given for sophomores, and culminating in a thorough study of the 
dynamics of a rigid body in two dimensions. This course may be 
followed by a half-course or a full course which begins with the 
kinematics and kinetics of a rigid body in three dimensions and 
proceeds to Lagrange's Equations and the variational principles. 
So important are Hamilton's Equations and their solution by 
means of Jacobi's Equation, that this subject has also been in- 
cluded. It appears that there is a special need for treating this 
theory, for although it is exceedingly simple, the current text- 
books are unsatisfactory. They assume an undefined knowledge 
of the theory of partial differential equations of the first order, but 
they do not show how the theory is applied. As a matter of fact, 
no theory of these equations at all is required for understanding 
the solution just mentioned. What is needed is the fact that 
Hamilton's Equations are invariant of a contact transformation. 
A simple proof is given in Chapter XIV, in which the method 
most important for the physicist, namely, the method of separating 
the variables, is set forth with no involved preliminaries. But 
even this proof may be omitted or postponed, and the student may 
strike in at once with Chapter XV. 

The concept of the vector is essential throughout Mechanics, 
but intricate vector analysis is wholly unnecessary. A certain 
minute amount of the latter is however helpful, and has been set 
forth in Appendix A. 

Appendix D contains a definitive formulation of a class of 
problems which is most important in physics, and shows how 
d'Alembert's Principle and Lagrange's Equations apply. It ties 
together the various detailed studies of the text and gives the 
reader a comprehensive view of the subject as a whole. 

The book is designed as a careful and thorough introduction to 
Mechanics, but not of course, in this brief compass, as a treatise. 
With the principles of Mechanics once firmly established and 
clearly illustrated by numerous examples the student is well 
equipped for further study in the current text-books, of which may 



viii PREFACE 

be mentioned : Routh : An Elementary Treatise on Rigid Dynamics 
and also Advanced Dynamics, by the same author; particularly 
valuable for its many problems. Webster, Dynamics good 
material, and excellent for the student who is well trained in the 
rudiments, but hard reading for the beginner through poor pre- 
sentation and lacunae in the theory ; Appell, Mecanique rationelle y 
vols. i and ii a charming book, which the student may open 
at any chapter for supplementary reading and examples. Jeans, 
Mechanics, may also be mentioned for supplementary exercises; 
as a text it is unnecessarily hard mathematically for the Sopho- 
more, and it does not go far enough physically for the upper- 
classmari. It is unnecessary to emphasize the importance of 
further study by the problem method of more advanced and 
difficult exercises, such as are found in these books. But to go 
further in incorporating these problems into the present work 
would increase its size unduly. 

It is not merely a formal tribute, but one of deep appreciation, 
which I wish to pay to The Macmillan Company and to The 
Norwood Press for their hearty cooperation in all the many dif- 
ficult details of the typography. Good composition is a distinct 
aid in setting forth the thought which the formulas are designed 
to express. Its beauty is its own reward. 

To his teacher, Benjamin Osgood Peirce, who first blazed the 
trail in his course, Mathematics 4, given at Harvard in the middle 
of the eighties the Author wishes to acknowledge his profound 
gratitude. Out of these beginnings the book has grown, developed 
through the Author's courses at Harvard, extending over more 
than forty years, and out of courses given later at The National 
University of Peking. May it prove a help to the beginner in 
his first approach to the subject of Mechanics. 

WILLIAM FOGG OSGOOD 

May 1937 



CONTENTS 

CHAPTER I 

STATICS OF A PARTICLE 

PAGE 

1. Parallelogram of Forces 1 

2. Analytic Treatment by Trigonometry 3 

3. Equilibrium. The Triangle of Forces. Addition of Vectors . 4 

4. The Polygon of Forces 7 

5. Friction 9 

6. Solution of a Trigonometric Equation. Problem 12 

Exercises on Chapter I 15 

CHAPTER II 

STATICS OF A RIGID BODY 

1. Parallel Forces in a Plane 21 

2. Analytic Formulation ; n Forces 23 

3. Centre of Gravity 26 

4. Moment of a Force 28 

5. Couples in a Plane 29 

6. Resultant of Forces in a Plane. Equilibrium 32 

7. Couples in Space 34 

8. Resultant of Forces in Space. Equilibrium 36 

9. Moment of a Vector. Couples 37 

10. Vector Representation of Resultant Force and Couple. Resul- 

tant Axis. Wrench 38 

11. Moment of a Vector about a Line 40 

12. Equilibrium 41 

13. Centre of Gravity of n Particles 42 

14. Three Forces 43 

Exercises on Chapter II 46 

CHAPTER III 

MOTION OF A PARTICLE 

1. Rectilinear Motion 49 

2. Newton's Laws of Motion 50 

3. Absolute Units of Force 55 

4. Elastic Strings 58 

ix 



x CONTENTS 

PA OB 

5. A Problem of Motion 60 

6. Continuation; the Time 63 

7. Simple Harmonic Motion 64 

8. Motion under the Attraction of Gravitation 69 

9. Work Done by a Variable Force 72 

10. Kinetic Energy and Work 75 

11. Change of Units in Physics 76 

12. The Check of Dimensions 79 

13. Motion in a Resisting Medium 81 

14. Graph of the Resistance ; 84 

15. Motion in a Plane and in Space 86 

16. Vector Acceleration 90 

17. Newton's Second Law 92 

18. Motion of a Projectile 93 

19. Constrained Motion 95 

20. Simple Pendulum Motion 97 

21. Motion on a Smooth Curve 99 

22. Centrifugal Force 101 

23. The Centrifugal Oil Cup 105 

24. The Centrifugal Field of Force 106 

25. Central Force 108 

26. The Two Body Problem 114 

27. The Inverse Problem to Determine the Force 114 

28. Kepler's Laws 115 

29. On the Notion of Mass 118 



CHAPTER IV 

DYNAMICS OF A RIGID BODY 

1. Motion of the Centre of Gravity 120 

2. Applications 123 

3. The Equation of Moments 126 

4. Rotation about a Fixed Axis under Gravity 127 

5. The Compound Pendulum 130 

6. Continuation. Discussion of the Point of Support .... 132 

7. Kater's Pendulum 133 

8. Atwood's Machine 134 

9. The General Case of Rotation about a Point 136 

10. Moments of Inertia 137 

11. The Torsion Pendulum 139 

12. Rotation of a Plane Lamina, No Point Fixed 139 

13. Examples 141 



CONTENTS xi 

PAGE 

14. Billiard Ball, Struck Full 143 

15. Continuation. The Subsequent Motion ........ 145 

16. Further Examples 146 

Exercises on Chapter IV 151 

CHAPTER V 

KINEMATICS IN TWO DIMENSIONS 

1. The Rolling Wheel ' 154 

2. The Instantaneous Centre 155 

3. Rotation about the Instantaneous Centre 157 

4. The Centrodes 159 

5. Continuation. Proof of the Fundamental Theorem .... 162 

6. The Dancing Tea Cup 165 

7. The Kinetic Energy of a Rigid System 166 

8. Motion of Space with One Point Fixed 168 

9. Vector Angular Velocity 170 

10. Moving Axes. Proof of the Theorem of 8 172 

11. Space Centrode and Body Centrode 174 

12. Motion of Space. General Case 175 

13. The Ruled Surfaces 176 

14. Relative Velocities 177 

15. Proof of the Theorem of 12 179 

16. Lissajou's Curves 182 

17. Continuation. The General Case. The Commensurable Case. 

Periodicity 186 

Professor Sabine's Tracings of Lissajou's Curves 

between pages 190-191 

CHAPTER VI 

ROTATION 

1. Moments of Inertia 191 

2. Principal Axes of a Central Quadric 194 

3. Continuation. Determination of the Axes 196 

4. Moment of Momentum. Moment of a Localized Vector . . 197 

5. The Fundamental Theorem of Moments 199 

6. Vector Form for the Motion of the Centre of Mass .... 201 

7. The Invariable Line and Plane 201 

8. Transformation of 202 

9. Moments about the Centre of Mass 204 

10. Moments about an Arbitrary Point 205 



xii CONTENTS 

PAGE 

11. Moments about the Instantaneous Centre 207 

12. Evaluation of a for a Rigid System ; One Point Fixed ... 208 

13. Euler's Dynamical Equations 210 

14. Motion about a Fixed Point 212 

15. Euler's Geometrical Equations 214 

16. Continuation. The Direction Cosines of the Moving Axes . . 216 

17. The Gyroscope 217 

18. The Top 220 

19. Continuation. Discussion of the Motion 222 

20. Intrinsic Treatment of the Gyroscope 225 

21. The Relations Connecting v, F, and K 229 

22. Discussion of the Intrinsic Equations 231 

23. Billiard Ball 237 

24. Cartwheels 241 

25. R&ume* 245 

CHAPTER VII 
WORK AND ENERGY 

1. Work 248 

2. Continuation : Curved Paths 250 

3. Field of Force. Force Function. Potential 253 

4. Conservation of Energy 256 

5. Vanishing of the Internal Work for a Rigid System .... 258 

6. Kinetic Energy of a Rigid Body 260 

7. Final Definition of Work 261 

8. Work Done by a Moving Stairway 264 

9. Other Cases in Which the Internal Work Vanishes .... 266 
10. Work and Energy for a Rigid Body 266 

CHAPTER VIII 
IMPACT 

1. Impact of Particles 270 

2. Continuation. Oblique Impact 274 

3. Rigid Bodies 277 

4. Proof of the Theorem 279 

5. Tennis Ball, Returned with a Lawford 282 

CHAPTER IX 
RELATIVE MOTION AND MOVING AXES 

1. Relative Velocity 285 

2. Linear Velocity in Terms of Angular Velocity 285 



CONTENTS xiii 

PAGE 

3. Acceleration 287 

4. The Dynamical Equations 290 

5. The Centrifugal Field 291 

6. Foucault Pendulum 292 

CHAPTER X 
LAGRANGE'S EQUATIONS AND VIRTUAL VELOCITIES 

1. The Problem 297 

2. Lagrange's Equations in the Simplest Case 299 

3. Continuation. Particle on a Fixed or Moving Surface . . . 303 

4. The Spherical Pendulum 306 

5. Geodesies 308 

6. Lemma 310 

7. Lagrange's Equations in the General Case 312 

8. Discussion of the Equations. Holonomic and Non-Holonomic 

Systems 313 

9. Continuation. The Forces 315 

10. Conclusion. Lagrange's Multipliers 316 

11. Virtual Velocities and Virtual Work 318 

12. Computation of Q r 320 

13. Virtual Velocities, an Aid in the Choice of the TT T 321 

14. On the Number m of the Q T 322 

15. Forces of Constraint 325 

16. Euler's Equations, Deduced from Lagrange's Equations . . . 325 

17. Solution of Lagrange's Equations 326 

18. Equilibrium 330 

19. Small Oscillations 333 

Exercises on Chapter X 336 

CHAPTER XI 
HAMILTON'S CANONICAL EQUATIONS 

1. The Problem 338 

2. A General Theorem 339 

3. Proof of Hamilton's Equations 342 

CHAPTER XII 
D'ALEMBERT'S PRINCIPLE 

1. The Problem 345 

2. Lagrange's Equations for a System of Particles, Deduced from 

d'Alembert's Principle 348 

3. The Six Equations for a System of Particles, Deduced from 

d'Alembert's Principle 349 



riv CONTENTS 

PAGE 

4. Lagrange's Equations in the General Case, and d'Alembert's 

Principle 350 

5. Application : Euler's Dynamical Equations 352 

6. Examples 353 

CHAPTER XIII 

HAMILTON'S PRINCIPLE AND THE PRINCIPLE OF 
LEAST ACTION 

1. Definition of 5 356 

2. The Integral of Rational Mechanics 360 

3. Application to the Integral of Kinetic Energy 362 

4. Virtual Work 364 

5. The Fundamental Equation 364 

6. The Variational Principle 370 

7. Hamilton's Principle 370 

8. Lagrange's Principle of Least Action 372 

9. Jacobi's Principle of Least Action 377 

10. Critique of the Methods. Retrospect and Prospect .... 379 

11. Applications 379 

12. Hamilton's Integral a Minimum in a Restricted Region . . . 381 

13. Jacobi's Integral a Minimum in a Restricted Region .... 386 

CHAPTER XIV 

CONTACT TRANSFORMATIONS 

1. Purpose of the Chapter 389 

2. Integral Invariants 392 

3. Consequences of the Theorem 395 

4. Transformation of Hamilton's Equations by Contact Trans- 

formations 400 

5. Particular Contact Transformations 403 

6. Theft-Relations 407 

CHAPTER XV 

SOLUTION OF HAMILTON'S EQUATIONS 

1. The Problem and Its Treatment 410 

2. Reduction to the Equilibrium Problem 413 

3. Example. Simple Harmonic Motion 415 

4. H, Independent of t. Reduction to the Form, H' = Pi . . . 420 

5. Examples. Projectile in vacuo 424 



CONTENTS xv 

PAGE 

6. Comparison of the Two Methods 429 

7. Cyclic Coordinates 430 

8. Continuation. The General Case 433 

9. Examples. The Two-Body Problem 434 

10. Continuation. The Top 438 

11. Perturbations. Variation of Constants 440 

12. Continuation. A Second Method 444 

APPENDIX 

A. Vector Analysis 447 

B. The Differential Equation : (du/dt) z = f(u) 456 

C. Characteristics of Jacobi's Equation 466 

D. The General Problem of Rational Mechanics 476 

INDEX . . . . 491 



MECHANICS 

CHAPTER I 

STATICS OF A PARTICLE 

1. Parallelogram of Forces. By a force is meant a push or a 
pull. A stretched elastic band exerts a force. A spiral spring, 
like those used in the upholstered seats of automobiles, when 
compressed by a load, exerts a force. The earth exerts a force 
of attraction on a falling rain drop. 

The effect of a force acting at a given point, 0, depends not 
merely on the magnitude, or intensity, of the force, but also on 
the direction in which it acts. Lay off a right line from 
O in the direction of the force, and mpke the length of ^ ^ 
the line proportional to the intensity of the force ; for p JG 1 
example, if F is 10 Ibs., the length may be taken as 
10 in., or 10 cm., or more generally, ten times the length which 
represents the unit force. Then this directed right line, or vector, 
gives a complete geometric picture of the force. Thus if a barrel 
of flour is suspended by a rope (and is at rest), the attraction of 
gravity the pull of the earth will be represented by a vector 
pointing downward and of length W, the weight of the barrel. 
On the other hand, the force which the rope exerts on the barrel 
will be represented by an equal and opposite vector, pointing 
upward. For, action and reaction are equal and opposite. 
When two forces act at a point, they are 
equivalent to a single force, which is found as 
follows. Lay off from the point the two vec- 
tors, P and Q, which represent the given forces, 
and construct the parallelogram, of which the 
Fia 2 right line segments determined by P and Q are 

two adjacent sides. The diagonal of the paral- 
lelogram drawn from determines a vector, R, which represents 

1 





2 MECHANICS 

the combined effect of P and Q. This force, R, is called the 
resultant of P and Q, and the figure just described is known as the 
parallelogram offerees. 

Example 1. Two forces of 20 pounds each make an angle of 
60 with each other. To find their resultant. 

Here, it is obvious from the geometry of the 
figure that the parallelogram is a rhombus, and 
that _the length of the diagonal in question is 
20 N/3 = 34.64. Hence the resultant is a force of 
34.64 pounds, its line of action bisecting the angle between the 
given forces. 

Example 2. Two forces of 7 pounds and 9 pounds act at a 
point and make an angle of 70 with each other. To find their 
resultant. 

Graphical Solution. Draw the forces to scale, constructing the 
angle by means of a protractor. Then complete the parallelo- 
gram and measure the diagonal. Find its direction with the 
protractor. 

Example 3. A picture weighing 15 Ibs. hangs from a nail in 
the wall by a wire, the two segments of which make angles of 30 
with the horizon. Find the tension in the wire. 

Here, the resultant, 15, of the two unknown tensions, T and T 9 
is given, and the angles are known. It is evident from the figure 
that T also has the value 15. So the answer is : 15 Ibs. 

Decomposition of Forces. Conversely, a given force can be de- 
composed along any two directions whatever. All that is needed 
is, to construct the parallelogram, of which the given force is 
the diagonal and whose sides lie along the given lines. 




FBlTKf, 



FIG. 4 FIG. 5 

If, in particular, the lines are perpendicular to each other, 
the components will evidently be : 

F cos <p, F sin <p. 



STATICS OF A PARTICLE 3 

EXERCISES 

1. Two forces of 5 Ibs. and 12 Ibs. make a right angle with 
each other. Show that the resultant force is 13 Ibs. and that it 
makes an angle of 22 37' with the larger force. 

2. Forces of 5 Ibs. and 7 Ibs. make an angle of 100 with each 
other. Determine the resultant force graphically. 

3. If the forces in Question 1 make an angle of 60 with each 
other, find the resultant. 

Give first a graphical solution. Then obtain an analytical 
solution, using however no trigonometry beyond a table of natural 
sines, cosines, and tangents. 

4. If two forces of 12 Ibs. and 16 Ibs. have a resultant of 20 Ibs., 
what angle must they make with each other and with the resultant? 

5. A force of 100 Ibs. acts north. Resolve it into an easterly 
and a north-westerly component. 

6. A force of 50 Ibs. acts east north-east. Resolve it into an 
easterly and a northerly component. Ans. 46.20 Ibs. ; 19.14 Ibs. 

7. A force of 12 Ibs. acts in a given direction. Resolve it into 
two forces that make angles of 30 and 40 with its line of action. 
Only a graphical solution is required. 

2. Analytic Treatment by Trigonometry. The problem of 
finding the resultant calls for the determination of one side of a 
triangle when the other two sides and the included angle arc 
known; and also of finding the remaining angles. The first 
problem is solved by the Law of Cosines in Trigonometry : 
(1) c 2 = a 2 + 6 2 - 2ab cos C. 

Here, a = P, b = Q, c = R, 




C = 180 - w 
and hence c 

(2) 72 2 = P 2 + Q 2 + 2PQ cos co. FIG. 

Example. Forces of 5 Ibs. and 8 Ibs. make an angle of 120 
with each other. Find their resultant. Here, 

R 2 = 25 + 64 - 2 X 5 X 8 X = 49 ; 
R = 7 Ibs. 

To complete the solution and find the remaining angles we 
can use the Law of Sines : 



4 MECHANICS 

~ I, 

(3) 

1 
(4) 



sin A sin B sin C 
Thus 



sm ^> sm 



There is no difficulty here about the sign when the adjacent 
angle is used, since sin (180 to) = sin co. 

In the numerical example above, Equation (4) becomes : 

8 7 



sin <p |\/3 
Thus 

sin <p = 4-V3, cos <p = | , <t> = 81 47'. 

The third angle is found from the fact that the sum of the 
angles of a triangle is two right angles : 

A + B + C = 180. 

To sum up, then : Compute the resultant by the Law of Cosines 
and complete the solution by the Law of Sines. 

EXERCISES 

Give both a graphical and an analytical solution each time. 

1. Forces of 2 Ibs. and 3 Ibs. act at right angles to each other. 
Find their resultant in magnitude and direction.* 

2. Forces of 4 Ibs. and 5 Ibs. make an angle of 70 with each 
other. Find their resultant. 

3. Equilibrium. The Triangle of Forces. Addition of Vec- 
tors. In order that three forces be in equilibrium, it is clearly 
necessary and sufficient that any one of them be equal and opposite 
to the resultant of the other two. The condition can be expressed 
conveniently by aid of the idea of the addition of vectors. 

First of all, two vectors are defined as equal if they have the 
same magnitude, direction, and sense, no matter where in the 
plane (or in space) they may lie. 

* Observe that in this case it is easier to determine the angle from its tangent. 
Square roots should be computed from a Table of Square Roots. Huntington's 
Four-Place Tables are convenient, and are adequate for the ordinary cases that 
arise in practice. But cases not infrequently arise in which more elaborate tables 
are needed, and Barlow's will be found useful. 




STATICS OF A PARTICLE 5 

Vector Addition. Let A and B be any two vectors. Construct 
A with any point, 0, as its initial point. Then, with the terminal 
point of A as its initial point, construct B. The vector, C, whose 
initial point is the initial point of A and whose terminal point 
is the terminal point of B, is defined as the vector 
sum, or, simply, the sum of A and B : 

C = A + B. 

It is obvious that 

B + A = A + B. 

Any number of vectors can be added by applying the definition 
successively. It is easily seen that 

(A + B) + C = A + (B + C). 
Consequently the sum 

A! + A 2 + - - - + A n 

is independent of the order in which the terms are added. 

For accuracy and completeness it is necessary to introduce the 
nil vector. Suppose, for example, that A and B are equal and 
opposite. Then their sum is not a vector in any sense as yet 
considered, for the terminal point coincides with the initial point. 
When this situation occurs, we say that we have a nil vector, and 
denote it by : 

A + B = 0. 

We write, furthermore,* 

B =- A. 

Equilibrium. The condition, necessary and sufficient, that 
three forces be in equilibrium is that their vector sum be 0. Geo- 
metrically this is equivalent to saying that the vectors which 
represent the forces can be drawn so that the fig- 
ure will close and form a triangle. From the Law 
of Sines we have : 

P Q _ E 




sin p sin q sin e 
FIG. 8 " p + q + e = 180. 

* It is not necessary for the present to go further into vector analysis than the 
above definitions imply. Later, the two forms of product will be needed, and 
the student may be interested even at this stage in reading Chapter XIII of the 
author's Advanced Calculus, or Appendix A. 



6 



MECHANICS 




FIG. 9 



Since sin (180 A) = sin 4, we can state the result in the 
following form. Let three forces, P, Q, and E, acting on a par- 
ticle, be in equilibrium. Denote the angles between 
the forces, as indicated, by p, q, e. Then Equa- 
tion (1) represents a necessary condition for equilib- 
rium. Conversely, this condition is sufficient. 

We thus obtain a convenient solution in all cases 
except the one in which the magnitudes of the forces, 
but no angles, are given. Here, the Law of Cosines * 
gives one angle, and then a second angle can be 
computed by the Law of Sines. 

Example 1. Forces of 4, 5, and 6 are in equilibrium. Find 
the angles between them. 

First, solve the problem graphically, measuring the angles. 
Next, apply the Law of Cosines : 

42 = 52 + 62 _ 2 X 5 X 6 X cos p, 

cos <p = f , <p = 41 23'. 

A second angle is now computed by the Law of Sines : 

5 4 



sin i 

5V7 
16 ' 



sin <p 



55 46'. 



The third angle is 82 51'. 

Example 2. A 40 Ib. weight rests on a smooth horizontal 
cylinder and is kept from slipping by a cord that passes over the 
cylinder and carries a 10 Ib. weight at its other 
end. Find the position of equilibrium. 

The cord is assumed weightless, and since it 
passes over a smooth surface, the tension in 
it is the same at all points. The surface of 
the cylinder is smooth, hence its reaction is 
normal to its surface. Let 6 be the unknown 
angle that the radius drawn to the weight FIG. 10 

* If we had a large number of numerical problems to solve, it would pay to use 
the more elaborate theorems of Trigonometry (e.g. Law of Tangents). But for 
ordinary household purposes the more familiar law is enough. 




STATICS OF A PARTICLE 



makes with the vertical. Then from inspection of the figure 
we see that 10 40 



or 



sin 6 sin 90' 

sin 6 = , = 14 29'. 

EXERCISES 



Find 




1. Forces of 7, 8, and 9 pounds keep a particle at rest, 
the angles they make with one another. 

2. Forces of 51.42, 63.81, and 71.93 grs. keep a particle at rest. 
What angle do the first two forces make with each other? Find 
the other angles. 

3. A weightless string passes over two smooth pegs at the same 
level and carries weights of P and P at its ends. In the middle, 
there is knotted a weight W. What 

angle do the segments of the string p 
make with the vertical, when the 
system is at rest ? w 

Ans. sin 6 -^ 

4. A boat is prevented from drifting down stream by two ropes 
tied to the bow of the boat, and to stakes at opposite points on the 
banks. One rope is 125 ft. long; the other, 150 ft.; and the 
stream is 200 ft. broad. If the tension in the shorter rope is 
20 Ibs., what is the tension in the other rope? 

6. Two smooth inclined planes, back to 
back, meet along a horizontal straight 
line, and make angles of 30 arid 45 with 
the horizon. A weight of 10 Ibs. placed 
on the first plane is held by a cord that 
passes over the top of the planes and 
carries a weight W, resting on the other plane and attached to 
the end of the cord. Find what value W must have. 

4. The Polygon of Forces. From the 
case of three forces the generalization to 
the case of n forces acting at a point pre- 
sents no difficulty. Add the forces geometri- 
cally, i.e. by the vector law. The vector 
sum represents the resultant of all n forces. 
Thus, in the figure, the resultant is given by FIG. 13 




FIG. 12 





8 MECHANICS 

the vector whose initial point is the point and whoso terminal 

point is P. 

The condition for equilibrium is clearly that the resultant be a 
nil vector, or that the broken line close 
and form a polygon but not necessarily 
a polygon in the sense of elementary 
geometry, since its sides may intersect, as 
in Figure 14. 

This condition will obviously be ful- 

filled if and only if the sum of the projections of the forces along 

each of two lines that intersect is zero.* 

Analytically, the resultant can be represented as follows. 

Let a Cartesian system of coordinates be assumed, and let the 

components of the force F k along the axes be X k and Y k . If, 

now, the components of the resultant are denoted by X and Y, 

we have : v _ v , v , , v 

A A! -\- A 2 ~r * ~r A n , 

Y = Y t + F 2 + + Y n . 
Such sums are written as 



(1) X*, or Xk > or Z *> 

t=l I 

depending on how elaborate the notation should be to insure 
clearness. 

The forces will be in equilibrium if, and only if, the resultant 
force is nil, and this will be the case if 

(2) 2) X k = 0, 2 Y k = 0. 

t-i t=i 

EXERCISE 

A 4 Ib. weight is acted on by three forces, all of which lie in the 
same vertical plane : a force of 10 Ibs. making an angle of 30 with 
the vertical, and forces of 8 Ibs. and 12 Ibs. on the other side of 
the vertical and making angles of 20 with the upward vertical 
and 15 with the downward vertical respectively. Find the force 
that will keep the system at rest. 

Space of Three Dimensions. If more than two forces act at a 
point, they need not lie in a plane. But they can be added two 

* Cf. Osgood and Graustein, Analytic Geometry, pp. 1-6. 



STATICS OF A PARTICLE 9 

at a time by the parallelogram law, the first two thus being 
replaced by a single force their resultant and this force in 
turn compounded with the third force; etc. The broken line 
that represents the addition of the vectors no longer lies in a plane, 
but becomes a skew broken line in space, and the polygon of forces 
becomes a skew polygon. The components of the resultant 
force along the three axes are : 

n n^ n 

(3) X = 2^ X^ Y = 2^ Yk, Z = 2^ Zk. 

The condition for equilibrium is : 

In all of these formulas, X k , Y k , Z k are algebraic quantities, 
being positive when the component has the sense of the positive 
axis of coordinates, and negative when tho sense is the opposite. 
In solving problems in equilibrium it is frequently simpler to single 
out the components that have one sense along the line in question 
and equate their sum, each being taken as positive, to the sum 
of the components in the opposite direction, each of these being 
taken as positive, also. The method will be illustrated by the 
examples in friction of the next paragraph. 

5. Friction. Let a brick be placed on a table ; let a string be 
fastened to the brick, and let the string be pulled horizontally with 
a force F just sufficient to move the brick. Then the law of 
physics is that A 

F = pR, R\ 

r J -p^ 
where R (here, the weight of the brick) is p 15 

the normal* pressure of the table on the 

brick, arid ju (the coefficient of friction) is a constant for the two 
surfaces in contact. Thus, if a second brick were placed on top 
of the first, R would be doubled, and so would F. 

We can state the law of friction generally by saying: When 
two surfaces are in contact and one is just on the point of slipping 

* Normal means, at right angles to the surface in question. The normal to a 
surface at a point is the line perpendicular to the tangent plane of the surface at 
the point in question. 




10 MECHANICS 

over the other, the tangential force F due to friction is propor- 
tional to the normal pressure R between the surfaces, or 



where /*, the coefficient of friction, is independent of F and R, 
and depends only on the substances in contact, but not on the 
area of the surfaces which touch each other. For metals on metals 
n usually lies between 0.15 and 0.25 in the case of statical fric- 
tion. For sliding friction /* is about 0.15; cf. Rankine, Applied 
Mechanics. 

A simple experiment often performed in the laboratory for 
determining /x is the following. Let one of the surfaces be repre- 
sented by an inclined plane, the angle of 
which can be varied. Let the other surface 
be represented by a rider, or small block of 
the substance in question, placed on the 
plane. If the plane is gradually tilted from 
a horizontal position, the rider will not slip 
for a time. Finally, a position will be reached 
for which the rider just slips. This angle of the plane is known as 
the angle of friction and is usually denoted by X. Let us show that 

n tan X. 

Resolve the force of gravity, W, into its two components along 
the plane and normal to the plane. These are : 

W sin X, W cos X. 

And now the forces acting up the plane (i.e. the components 
directed up the plane) must equal the forces down the plane, or 

F = W sin X ; 

and the forces normal to the .plane and upward must equal the 
forces normal to the plane and downward, or 

R = W cos X. 
Hence 

F sin X , x 
- = an ^ 

R cosX 
But 

F = /J2. 
Consequently 

n tan X. 





STATICS OF A PARTICLE 11 

Example. A 50 Ib. weight is placed on a rough inclined plane, 
angle of elevation, 30. A cord attached to the weight passes 
over a smooth pulley at the top of the plane and carries a weight W 
at its lower end. For what values of W will the system be in 
equilibrium if jut = -J ? 

Here, X < 30, and so, if W is very small, the 50 Ib. weight will 
slip down the plane. Suppose W is just large enough to prevent 
slipping. Then friction acts up the plane, and the forces which 
produce equilibrium are those indicated. Hence 



'F+W 

50 sin 30 
W 

50 cos 30 
Fio. 17 Fia. 18 

F + W = 50 sin 30 = 25, 
R = 50 cos 30 = 25 V3, 
and F = %R. 

It follows, then, that 

W = 6 ~ 25 = 17.8 Ibs. 
o 

If, now, W is slightly increased, the 50 Ib. weight will obviously 
still be in equilibrium, and this will continue to be the case until 
the 50 Ib. weight is just on the point of slipping up the plane. 
This will occur when W = 32.2 Ibs. as the student can now prove 
for himself. Consequently, the values of W for which there is 
equilibrium are those for which 

17.8 ^ W g 32.2. 

EXERCISES 

1. If the cylinder of Example 2, 3, is rough, /z = , find the 
total range of equilibrium. Ans. 4 49' g g 23 44'. 

2. Consider the inclined planes of Exercise 5, 3. If the one 
on which the 10 Ib. weight rests is rough, /z = T ^, find the range 
of values for W that will yield equilibrium. 



12 



MECHANICS 



3. Prove the formula 

H = tan X 

by means of the triangle of forces, i.e. the Law of Sines, 3, (1). 

6. Solution of a Trigonometric Equation. Problem. A 50 Ib. 

weight rests on a rough horizontal plane, ju = -. A cord is 
fastened to the weight, passes over a smooth pulley 2 ft. above 
the plane, and carries a weight of 25 Ibs. which hangs freely at 
its other end. To find all the positions of equilibrium. 
Resolving the forces horizontally and vertically, we find : 

25 cos 6 = R, 
25 sin + R = 50. 
Hence, eliminating R, we obtain 
the equation : 

FIG. 19 (1)6 cos 6 + sin = 2. 

This equation is of the form : 
(2) a cos + b sin = c, 

and is solved as follows. * Divide through by Va 2 + b 2 : 




50 



\OJ / COS -1 7= 

Vo2 _|_ ^2 Va 2 
and then set 

fA\ a 

(4; = = = cos a, 
Va 2 + b 2 

Thus 


SHI V jr-- ~~- ' 

b 


,- - - sin a. 
Va 2 + b 2 



cos a cos + sin a sin 6 = 



Va 2 + 6 2 ' 



or 
(5) 



cos (0 a) = 



Va 2 + b 2 



* The student should observe carefully the trigonometric technique set forth 
in this paragraph, not merely because equations of this type are important in them- 
selves, but because the practical value of a working knowledge of trigonometry 
is not confined to solving numerical triangles. Of far greater scope and importance 
in practice are the purely analytical reductions to other trigonometric foi-ms, and 
the solution of trigonometric equations. That is one of the reasons why the 
harder examples at the end of the chapter are valuable. They not only give 
needed practice in formulating mathematically physical data ; they require also 
the ability to handle analytical trigonometry according to the demands of practice. 



STATICS OF A PARTICLE 13 

The angle a is most easily determined from the equation : 
(6) 



Thus a is seen to be one of two angles which one is rendered 
clear by plotting the point on the unit circle : 

z 2 + 2/ 2 = 1, 
whose coordinates are 

= __JL__ 7 b __ 

x ' y ~ 



The angle from the positive axis of x to the radius drawn to this 
point is a. Thus we have a graphical determination of a. It is 
not necessary to compute the coordinates accurately, but merely 
to observe in which quadrant the point lies, so as to know which 
root of the equation for tan a to take. Thus if b > 0, a must be 
an angle of the first or second quadrant. Finally, if c/Va 2 + b 2 
is numerically greater than 1, the equation has no solution. 

In defining a, it would, of course, Jiave answered just as well if 
sin a and cos a had been interchanged, and if either or both the 
ratios in (4) had been replaced by their negative values.* 

Returning now to the numerical equation above, we see that 

tan a = , sin a > 0, a = 9 28' ; 

cos (6 - 9 280 - 



- 9 28' = 70 48'. 

Since 6 in the problem before us must be an angle of the first 
quadrant, the lower sign is impossible, and 

= 80 16'. 

We have determined the point of the plane at which all the 
friction is called into play and the 50 Ib. weight is just on the 
point of slipping. For other positions, F will not equal pR. 
Such a position will be one of equilibrium if the amount of friction 
actually called into play, or F, is less than the amount that could 

* Equation (2) might also have been solved by transposing one term from the 
left- to the right-hand side and squaring. On using the Pythagorean Identity : 

sin 2 -f cos 2 = 1, 

we should be led to a quadratic equation in the sine or cosine. This equation will, 
in general, have four roots between and 360, and three of them must be excluded. 
Moreover, the actual computation by this method is more laborious. 



14 MECHANICS 

be called into play, or pR. It seems plausible that such points lie 
to the right of the critical point ; but this conclusion is not im- 
mediately justified, for, although the amount of friction required, 

01 F = 25 cos B, 

is less for a larger 0, still, the amount available, or 

n 50-25 sin 
Mfi- - g - , 

is also less. We must prove, therefore, that 

F < nR 

or 

OK ^50-25 sin 

25 cos < - 5 -- 
b 

This will obviously be so if 

6 cos 6 < 2 - sin 0, 80 16' < < 90, 

or if 

6 cos + sin < 2, 

rif 6 1 2 



or if . 

cos (0 - 9 28 7 ) < 



-=' 



As 0, starting with the value 80 16', increases, 9 28' also 
increases, and consequently cos (0 9 28') decreases. Conse- 
quently our guess is borne out by the facts, and the 50 Ib. weight 
will be in equilibrium at all points on the table within a circle of 
radius .343 ft., or a little over 4 in., whose centre is directly under 
the pulley. 

EXERCISES 

1. Solve the same problem if the plane is inclined at an angle 
of 15 with the horizon, and the vertical plane through the weight 
and the pulley is at right angles to the rough plane. 

Ana. 43 33' g0g 69 24'. 

2. At what angle should the plane be tilted, in order that the 
region of equilibrium may just extend indefinitely down the plane? 

3. Find the angle of the third quadrant determined by the 

equation : n . 

M 3 sin 6 - 2 cos = 1. 



STATICS OF A PARTICLE 15 

4. Show that there are in all eight ways of solving Equation (2), 
given by setting the right-hand sides of Equations (4) equal to 
cos a, + sin a and sin a, cos a, where the signs are 
independent of each other. 

5. Evaluate the integral : 

dx 



s-. 




a cos x + b sin x 
6. Solve the equation : 

2 cos 2 <p 4 cos <p sin <p 3 sin 2 <p = 5. 
Suggestion. Introduce the double angle, 2<p. 

EXERCISES ON CHAPTER I* 

1. A rope runs through a block, to which another rope is 
attached. The tension in the first rope is 

120 Ibs., and the angle it includes is 70. 
What is the tension in the second rope ? 

2. A man weighing 160 Ibs. is lying in a 
hammock. The rope at his head makes an 
angle of 30 with the horizon, and the rope 

at his feet, an angle of 15. Find the tensions in the two ropes. 

3. A load of furniture is being moved. The rope that binds 
it passes over the round of a chair. The tension on one side of the 
round is 40 Ibs. and on the other side, 50 Ibs. ; and the angle is 
100. What force does the round have to withstand ? 

4. A canal boat is being towed by a hawser pulled by horses 
on the bank. The tension in the hawser is 400 Ibs. and it makes 

4 an angle of 15 with the bank. What is 

the effective pull on the boat in the direc- 
tion of the canal? 

5. A crane supports a weight of a ton 
as shown in the figure. What arc the 
forces in the horizontal and in the oblique 
FlG - 21 member? 

6. Three smooth pulleys can be set at pleasure on a horizon- 
tal circular wire. Three strings, knotted together, pass over the 

* The student should begin each time by drawing an adequate figure, illustrating 
the physical objects involved, and he should put in the forces with colored ink or 
pencil. A bottle of red ink, used sparingly, contributes tremendously to clear 
thinking. 




16 



MECHANICS 



pulleys and carry weights of 7, 8, and 9 Ibs. at their free ends. 

How must the pulleys be set, in order that the knot may be at 

rest at the centre of the circle ? 

7. A telegraph pole at two cross- 
roads supports a cable, the tension 
in which is a ton. The cable lies in 
a horizontal plane and is turned 
through a right angle at the pole. 
The pole is kept from tipping by a 




FIG. 22 




FIG. 23 




stay from its top to the ground, the stay 
making an angle of 45 with the verti- 
cal. What is the tension in the stay? 

8. The figure suggests a stake of a 
circus tent, with a tension of 500 Ibs. 
to be held. What is the tension in 
the stay, if the stake could turn freely? 

9. Two men are raising a weight of 150 Ibs. by a rope that 

passes over two smooth pulleys and is 
knotted at A. How hard are they 
pulling? 

10. If, in the preceding question, in- 
stead of being knotted at A, the two 
ropes the men have hold of passed over 
pulleys at A and were vertical above A, 
how hard would the men then have to 
pull? 

11. A weight W is placed in a smooth hemispherical bowl ; a 
string, attached to the weight, passes over the edge of the bowl 
and carries a weight P at its other end. Find the position of 
equilibrium. 

12. Solve the same problem for a parabolic bowl, the rim being 
at the level of the focus. 

13. One end of a string is made fast to a peg at A. The string 
passes over a smooth peg at J?, at the same level as A, and carries a 
weight P at its free end. A smooth heavy bead, of weight W, can 
slide on the string. Find the position of equilibrium and the 
pressure on the peg at B. 

14. A bead weighing W Ibs. can slide on a smooth vertical 
circle of radius a. To the bead is attached a string that passes 



FIG. 24 



STATICS OF A PARTICLE 17 

over a smooth peg situated at a distance %a above the centre of 
the circle, and has attached to its other end a weight P. Find 
all the positions of equilibrium. 

16. A 50 Ib. weight rests on a smooth inclined plane (angle 
with the horizontal, 20) and is kept from slipping by a cord which 
passes over a smooth peg 1 ft. above the top of the plane, and 
which carries a weight of 25 Ibs. at its other end. Find the 
position of equilibrium. 

16. A heavy bead can slide on a smooth wire in the form of a 
parabola with vertical axis and vertex at the highest point, A 
string attached to the bead passes over a smooth peg at the focus 
of the parabola and carries a weight at its other end. Show that 
in general there is only one position of equilibrium ; but some- 
times all positions are positions of equilibrium. 

17. A weightless bead * can slide on a smooth wire in the form 
of an ellipse whose plane is vertical. A string is knotted to the 
bead and passes over two smooth pegs at the foci, which are at 
the same horizontal height. Weights of P and Q f iro attached 
to the two ends of the string. Find the positions of equilibrium. 

18. An inextensible flexible string has its ends made fast at two 
points and carries a weightless smooth bead. Another string is 
fastened to the bead and drawn taut. Show that every position 
of the bead is one of equilibrium, if the second string is properly 
directed. 

19. Give a mechanical proof, based on the preceding question, 
that the focal radii of an ellipse make equal angles with the tangent. 

20. A bead of weight P can slide on a smooth, vertical rod. 
To the bead is attached an inextensible string of length 2a, 
carrying at its middle point a weight W and having its other end 
made fast to a peg at a horizontal distance a from the rod. Show 
that the position of equilibrium is given by the equations : 

P tan <p = (P + W} tan 6, sin + sin <p = 1, 

where 0, <p are the angles the segments of the string make with 
the vertical. 

* Questions of this type may be objected to on the ground that a force must act 
on mass, and so there is no sense in speaking of forces which act on a masslcss ring. 
But if the ring has minute mass, the difficulty is removed. The problem may be 
thought of, then, as referring to a heavy bead, whose weight is just supported by 
a vertical string. Since the weight of the bead now has no influence on the position 
of equilibrium, the mass of the bead may be taken as very small, and so, physically 
negligible. 



18 MECHANICS 

21. If, in the preceding question, P = W y show that = 21 55', 
V = 38 49'. Determine these angles when W = 2P. 

22. A flexible inextensible string in the form of a loop 60 in. 
long is laid over two smooth pegs 20 in. apart and carries two 
smooth beads of weight P and W. Find the position of equi- 
librium, if the beads cannot come together. 

Ans. W sin 6 = P sin ^>, 

cos 6 + cos (f> = 3 cos 6 cos p ; 

cos 4 e - | cos 3 e - I (i - ~) cos 2 e 

2 



hence 

9 cos 4 6 - 6 cos 3 6 - 8\ cos 2 8 + 6X cos 6 - X = 0, 

where _ (W 2 - P 2 ) 

X ~ TP 

23. Show that if, in the preceding question, P = 5 and 
TF = 10, = 25 8', and find the reaction on the peg. 

24. One end of an inextensible string a in. long is made fast to 
a peg A and at the other end is knotted a weight W. A second 
string, attached to W, passes over a smooth peg at B, distant 
b in. from A and at the same level, and carries a weight P at its 
other end. Find the position of equilibrium. 

If P = Wj how far below the level of the pegs will the first 



^ - 25.* Observe the braces that stiffen the 

frame of a railroad car. Formulate a 

reasonable problem suggested by what you sec, and solve it. 

26. A bridge of simple type is suggested by the figure. In 

designing such a structure, the stiffness of the members at a point 

A B 



J_ 




FIG. 26 

* The following four problems are given only in outline, and the student thus 
has the opportunity of filling in reasonable numerical data and formulating a clean- 
cut question. It is not necessary that he respond to all the problems; but he 
should demand of himself that he develop a number of them and supplement these 
by others of like kind which he finds of his own initiative in everyday life. For, 
imagination is one of the highest of the intellectual gifts, and too much effort 
cannot be spent in developing it. 



STATICS OF A PARTICLE 19 

where these come together is not to be utilized, but the frame is 
planned as if the members were all pivoted there. Draw such a 
bridge to scale and find what the tensions and thrusts will be if 
it is to support a weight of 20 tons at each of the points A, B. 
Make a reasonable assumption about the weight of the road bed, 
but neglect the weight of the tie rods, etc. j 100 lbs< 



27. The tension in each of the traces attached to _j_ Jo , 

o 



100 Ibs. 



a whiffle-tree 3 ft. long is 100 Ibs. The distance from 1( j 
the ring to the whifflc-tree is 10 in. What is the ten- 
sion in the chains ? Fm - 27 

28. Have you ever seen a funicular a small passenger car, 
hauled up a steep mountain by a cable? How is the tension in 
tho cable related to the weight of the car? When the direction 
of the cable is changed by a friction pin, or roller, over which the 
cable passes, what is the pressure on the pin? 

FRICTION 

29. Consider the inclined planes of Question 5, 3. If both 
.ire rough and /z = -fa for each, what is the range of values for W 
consistent with equilibrium? 

30. A weightless bead can slide on a rough horizontal wire, 
ju = 0.1. A cord is attached to the bead and carries a weight at 
its other end, thus forming a simple pendulum. Through what 
angle can the pendulum swing without causing the bead to slip? 

31. A water main 5 ft. in diameter is filled with water to a 
depth of 1 ft. A mouse tumbles in and swims to the nearest point 
on the wall. If the coefficient of friction between her feet and the 
pipe is -J-, can she clamber up, or will she be drowned? 

32. A heavy bead is placed on a rough vertical circle, the 
coefficient of friction being f . If the angle between the radius 
drawn to the bead and the vertical is 16, find whether the bead 
will slip when released. 

33. A rope is fastened to a weight that rests on a rough hori- 
zontal plane, and pulled until the weight just moves. Find the 
tension in the rope, and show that it will be least when the rope 
makes, with the horizontal, the angle of friction. 

34. The same question for an inclined plane. 



20 MECHANICS 

35. A 50 Ib. weight is placed on a rough inclined plane, M = t, 
angle of inclination, 10. A string tied to the weight passes over 
a smooth peg at the same level as the weight and carries a weight 
of 7 Ibs. at its lower end. When the system is released from rest, 
will it slip ? 

36. A weight is placed on a rough inclined plane and is attached 
to a cord, the other end of which is made fast to a peg in the plane. 
Find all positions of equilibrium. 

37. If the parabolic wire described in Question 16 is rough, and 
the weights are P and W, find all positions of equilibrium. 

Ans. When P ^ W, the limiting position is given by one or 
the other of the equations : 

i - P ~ W 1 ? - W ~ P 1 

tan 2 ~" P + W ' /z' tan 2 " W + P ' n' 

Find the other positions of equilibrium, and discuss the 
case P = W. 

38. Cast iron rings weighing 1 Ib. each can slide on a rough 
horizontal rod, M = -J. A string 6 ft. long is attached to each of 
these beads and carries a smooth bead weighing 5 Ibs. How far 
apart can the two beads on the rod be placed, if the system is to 
remain at rest when released ? 

39. An elastic string 6 ft. long, obeying Hooke's Law, is stretched 
to a length of 6 ft. 6 in. by a force of 20 Ibs. The ends of the 
string are made fast at two points 6 ft. apart and on the same 
level. A weight of 4 Ibs. is attached to the mid-point of the string 
and carefully lowered. Find the position of equilibrium, neglect- 
ing the weight of the string. Ans. is given by the equation : 

cot = 120 (1 - cos 0). 

40. Solve the preceding equation for 0, to one-tenth of a degree. 

Ans. = 14|. 

41. The mast of a derrick is 40 ft. high, and a stay is fastened 

^ 20 to a block of stone weighing 
4 tons and resting on a pave- 
ment, M = f The boom is 

35 ft. long, and its end is dis- 

oo tant 20 ft. from the top of the 

riG. &Q . 11- 

mast. Is it possible to raise 

a 5 ton weight, without the derrick's being pulled over, the dis- 
tance from the stone to the derrick being 120 ft.? 




CHAPTER II 



STATICS OF A RIGID BODY 

1. Parallel Forces in a Plane. Lot two parallel forces, P and 
Q, act on a body at A and B, and let them have the same sense. 
Introduce two equal and opposite forces, S and S', at A and B as 
shown in the figure, and, com- 
pounding them with P and Q 
respectively, carry the resulting 
forces back to the point D in 
which their lines of action meet. 
These latter forces are now seen 
to have a resultant, 

(1) R = P + Q, 

parallel to the given forces and 

having the same sense, its line 

of action dividing the line AB 

into two segments, AC and CB. Let the lengths of the segments 

be denoted as follows: AC = a, CB = 6, AB = c, DC = h. 

From similar triangles it is seen that 




fr I(3 29 



Hence 



P 

S 



h 
a' 



Q h 

AS' 6' 



aP = bQ. 



a + 6 = c. 



(2) 

Moreover, 

(3) 

To sum up, then : The original forces, P and Q, have a resultant 
determined by the equations (1), (2), and (3). 

Example. The familiar gravity balance, in which one arm, a, 
from which the weight P to be determined 
is suspended, is short, and the other arm, b, 
from which the rider Q hangs is long, is a 
FIG. 30 case in point. 

21 




22 



MECHANICS 



Q 



1 



Opposite Forces. If P and Q are opposite in direction, and 
unequal (Q > P, say), they also have a resultant. Introduce a 
force E (Equilibriant) parallel to P and Q and having the sense 
of P, determining it so that Q will be equal and opposite to the 
resultant of P and E. Then 

Q = P + E, 
cP - bE, 

a = b + c. 

Thus P and Q are seen to have 
a resultant, 

FlG - 31 (4) R = Q - P, 

having the sense of Q, its line of action cutting AC produced in 
the point B determined by the equations : 

(5) aP = bQ, 

(6) a = b + c. 

If P and Q are equal, they form a couple and, as we shall show 
later, cannot be balanced by a single force; i.e. they have no 
resultant (force). 

Example. Consider a pair of nut crackers. The forces that 
act on one of the members are i) P, the pull of the hinge ; if) Q, 
the pressure of the nut; and Hi) the 
force E the hand exerts, balancing the 
resultant, R, of P and Q. 

We have here made use of the so-called 
Principle of the Transmissibilily of Force, 
which says that the effect of a force on a 
body is the same, no matter at what 
point in its line it acts. Thus a service 
truck will tow a mired car as effectively 
(but no more effectively) when the tow-rope is long, as when 
it is short, provided that in each case the rope is parallel to the 
road bed. 

Moreover, it is not necessary to think of the point of application 
as lying in the material body. It might be the centre of a ring. 
For we can always imagine a rigid weightless truss attached to the 
body and extending to the desired point. But we always think 
of a body, i.e. mass, on which the system of forces in question acts. 




FIG. 32 



STATICS OF A RIGID BODY 23 

EXERCISES 

1. A 10 ton truck passes over a bridge that is 450 ft. long. 
When the truck is one-third of the way over, how much of the 
load goes to one end of the bridge, and how much to the other 
end? Ans. 6f tons to the nearer end. 

2. A weight of 200 Ibs. is to be raised by a lever 6 ft. long, the 
fulcrum being at one end of the lever, and the weight distant 9 in. 
from the fulcrum. What force at the other end is needed, if the 
weight of the lever is negligible? 

3. A coolie carries two baskets of pottery by a pole 6 ft. long. 
If one basket weighs 50 pounds and the other, 70 pounds, how far 
arc the ends of the pole from his shoulder? 

2. Analytic Formulation ; n Forces. Suppose that n parallel 
forces act. Then two, which are not equal and opposite, can be 
replaced by their resultant, and this in turn combined with a third 
one of the given forces, until the number has been reduced to two. 
These will in general have a resultant, but, in particular, may form 
a couple or be in equilibrium. Thus the problem could be solved 
piecemeal in any given case. 

An explicit analytic solution can be obtained as follows. Begin 
with n = 2 and denote the forces by P l and P 2 . Moreover, let P 1 
arid P 2 be taken as algebraic quan- 
tities, being positive if they act in 
one direction ; negative, if they act p \ 

in the opposite direction. - - 1 - 

AT 1 T VI* XssQ 3J=1 ** *2 

Next draw a line perpendicular* Fl(J 33 

to the lines of action of P 1 and 

P 2 , and regard this line as the scale of (positive and negative) 
numbers, like the axis of x. Let x lf x 2 be the coordinates of the 
points in which P 1? P 2 cut the line. We proceed to prove the 
following theorem. 

The forces P l and P 2 have a resultant, 

(l) R = P, + P 

provided P l + P 2 ^ 0. Its line of action has the coordinate: 



* An oblique direction could be used, but in the absence of any need for such a 
generalization, the orthogonal direction is more concrete. 



24 MECHANICS 

Suppose, first, that P t and P 2 are both positive. Then, by 1, 
R = P, + P 2 



, 

where 

a = x x 1? o = x 2 x, 

provided Xj < x 2 (algebraically). Hence 

(x - x,) P l = (x 2 - x) P 2 , 

and from this equation, the relation (2) follows at once. 

The case that x 2 < x l is dealt with in a similar manner, as is also 
the case that P l and P 2 are both negative. 

Next, suppose P 1 and P 2 have opposite senses, but 

P l + P, * 0. 
Let P 1 < 0, P 2 > 0, | P 1 | < P 2 , 

where | x | means the numerical or absolute value of x. Thus 
| - 3 | = 3, | 3 | = 3. Moreover, let x l < x 2 . Then, by 1, 
P l and P 2 have a resultant, 

12 = -?! + P 2 , 

and the coordinate, x, corresponding to it is obtained as follows : 

a = x x lt b = x x tl 

and hence, from 1, (5) : 

(x - x { ) (- P t ) = (x - x 2 ) P 2 . 



So again we arrive at the same formulas, (1) and (2), as the 
solution of the problem. 

It remains merely to treat the remaining cases in like manner. 
The final result will always be expressed by formulas (1) and (2). 
We are now ready to proceed to the general case. 

THEOREM 1. Let n parallel forces, P lt , P n , act. They will 
have a resultant, 

R = P! ^ ---- + P n , 

provided this sum ^ 0, and its line of action will correspond to x, 
where 

/o\ ;= _ P\ X l i" * ' ' "T Pn X n 

(3) x - 



STATICS OF A RIGID BODY 25 

The proof can be given by the method of mathematical induc- 
tion. The theorem is known to be true for n = 2. Suppose 
it were not true for all values of n. Let m be the smallest value 
of n for which it is false. We now proceed to deduce a con- 
tradiction. 

Suppose, then, that P D - , P m is a system of parallel forces, 
for which the theorem is false, although it is true for n 2, 
3, , m - 1. By hypothesis, 

Pi + ' + Pm * 0. 

Now, it is possible to find m 1 of the P, 's whose sum is not : 

Pi + ' + Pm-, * 0, 

let us say. These m I forces have, by hypothesis, a resultant : 

R' = P l + - - + P w - lf 
and its x has the value : 

_/ /I 3*i r * ' " 'T~ -* w i #w~i 

x ~ />! + -TP^; ' 

since the theorem holds by hypothesis for all values of n < m. 
Next, combine this force with P w . Since 

R' + P m = 1\ + - - - + P m * 0, 
the two forces have a resultant, 

R = R' + P m = P 1 + - - + P w , 
and its line of action is given by the equation 

_ R'x' + P m x m P lgl + +P w a, 
X #' + P M A + --+P 

But this result contradicts the assumption that the theorem is 
false for n = m. Hence the theorem is true for all values of n. 

Couples. Let 

(4) P, + - - - + P n = 0, P n * 0. 

Thei1 P l + - + Pn-! ^ 0, 

and the forces P lf , P n _ 1 have a resultant, 

ft' = P 4- ... 4- P 

^ i r n^ * n 1> 

whose line of action is given by the equation : 

-/ = P! %l H~ ' ' "T Pn-i ^n~i 



26 MECHANICS 

If, in particular, x' = x n , this resultant, 72', will have the same 
line of action as P n ; and since 

R' + P n = 0, or R f = - P n , 
the n forces will be in equilibrium. We then have : 

_ PI X \ I ' ' ~T 1 n-i X n -i 
Xn r> y 

f n 

(5) Pl*l + ' + PnX n = 0. 



And conversely, if this condition holds, we can retrace our stops 
and infer equilibrium. But, in general, x' ^ x n . Hence 

_^ P, X l H ----- h Pn-i gn-i 
~ 



(6) Pl*l + ' ' +PnX n ^Q. 

We then have a couple. And conversely, if (4) and (6) hold, we 
can retrace our steps and infer that we have a couple. We have 
thus proved the following theorem. 

THEOREM 2. The n parallel forces P lt , P n form a couple if, 
arulonlyif PI + . . . + P. = 0. 



Equilibrium. The case of equilibrium includes not only the 
case above considered (P n ^ 0), but also the case in which all 
n forces vanish. We thus have the following theorem. 

THEOREM 3. The n parallel forces P ly , P n are in equilibrium 
if , and only if PI + . . . + Pn = ^ 

Pi X l + ---- h Pn X n = 0. 

3. Centre of Gravity. Let n particles, of masses Wi, , m n , 
be fastened to a rigid rod, the weight of which may be neglected, 
and let them be acted on by the force of gravity. If the rod is 
supported at a suitable point, (?, and is at rest, there will be no 
tendency to turn in any direction. This point is called the centre 
of gravity of the n particles, and its position is determined by the 
equation : 

m l x l + - + m n x n 



- 



m l + - + m n 



STATICS OF A RIGID BODY 27 

If the particles lie anywhere in a plane, being rigidly connected 
by a truss work of weightless rods, and if we denote the coordinates 
of m k by (xk, yk) 1 the centre of gravity is defined in a similar manner 
(sec below) and its coordinates, (x, ?/), are given by Equations 

(1) and 

/ 9 x fl _ *KI y\ H ---- + >n y n 

(2) y ~ n^ + .-.+m. ' 

For, let the plane of the particles be vertical, the axis of x being 
horizontal. Then the system is acted on by n parallel forces, 
whose lines of action cut the axis of x at right angles in the points 
%!,'', x ny and their resultant is determined in position by Equa- 
tion (1). On rotating the plane through a right angle and repeat- 
ing the reasoning, Equation (2) is obtained. 

The centre of gravity of any material system, made up of par- 
ticles and line, surface, and volume distributions, is defined as a 
point, (7, such that, if the parts of the system be rigidly connected 
by weightless rods, and if G be supported, there will be no tendency 
of the system to rotate, no matter how it be oriented. We have 
proved tho existence of such a point in the case of n particles 
lying on a line. For n particles in a plane we have assumed that 
a centre of gravity exists and lies in the plane, and then we have 
computed its coordinates. We shall prove later that n particles 
always have a centre of gravity, and that its coordinates are given 
by Equations (1), (2), and 



. . 

m l + + m n 

In the case of a continuous distribution of matter, like a tri- 
angular lamina or a solid hemisphere, the methods of the Calculus 
lead to the solution. It is the definite integral, defined as the 
limit of a sum, that is here employed, and Duhamel's Principle 
is essential in the formulation. In the simpler cases, simple 
integrals suffice. But even in some of these cases, surface and 
volume integrals simplify the computation. 

The following centres of gravity are given for reference. 
fl) Solid hemisphere : x = fa. 

b) Hemispherical surface : x a. 

c) Solid cone : x = f h. 

d) Conical surface : x f A. 

e) Triangle : Intersection of the medians. 



28 



MECHANICS 



4. Moment of a Force. Let F be a force lying in a given 
plane, and let be a point of the plane. By the moment of F about 
is meant the product of the force by the distance from of its 
line of action, or hF. A moment may furthermore be defined as 
an algebraic quantity, being taken as positive when it tends to turn 
the body in one direction (chosen arbitrarily as the positive 
direction), and negative in the other case. Finally, if lies on 
the line of action of the force, the moment is defined as 0. 

Let a force F act at a point (x, y), and let the components of F 
along the axes be denoted by X, Y. Then the moment (taken 
algebraically) of F about the origin, 0, is : 

(1) xY-yX. 

Proof. Let the equation of the line of action of F be written 
in Hesse's Normal Form : 

x cos a + y sin a = h. 




/ 




i FIG. 34 



O 
FIG. 35 



Suppose, first, that the moment is positive. Then it will be 

hF = x (F cos a) + y (F sin a). 
Here, 2ir a is the complement of 6, Fig. 34 : 



Hence 
and since 



cos a = sin 6, 



a = - + 2rr. 



sin a = cos 0, 



X = F cos 6, Y = F sin 6, 

the proof is complete. 



STATICS OF A RIGID BODY 29 

If, however, the moment is negative, a. and 6 will be connected 
by the relation, Fig. 35 : 

,- a --- Bt - + |. 

Hence 

cos a = sin 9, sin a = cos 6. 

The moment will now be repressed as 

hF = x ( F cos a) + y ( F sin a), 

and thus we arrive at the same expression, (1), as before. The same 
is true for a nil moment. Hence the formula (1) holds in all cases. 
From (1) we prove at once that the moment of the resultant of 
two forces acting at a point is the sum of the moments of the two 
given forces. Let the latter be Fj, F 2 , with the moments 

xY 1 yX l and xY 2 yX 2 . 

The components of the resultant force are seen to take the form : 
X l + X 2 and Y l + F 2 , and its moment is 



From this expression the truth of the theorem is at once obvious. 
Finally, the moment of a force about an arbitrary point, (x , ?/ ), 
is seen to be : 
(2) (x-x )Y-(y-y,}X. 

The physical meaning of the moment of a force about a point 
is a measure of the turning effect of the force. Suppose the body 
were pivoted at 0. Then the tendency to turn about 0, due to 
the force F, is expressed quantitatively by the momenta And a 
set of forces augment or reduce one another in their combined 
turning effect according to the magnitude and sense of the sum 
of the moments of the individual forces. From this point of view 
a moment is often described in physics and engineering as a torque. 

6. Couples in a Plane. A couple has already been defined as 
a system of two equal and opposite parallel forces. A couple 
cannot be balanced by a single force, but is an independent me- 
chanical entity ; the proof is given below. 

By the moment of a couple, taken numerically, is meant the 
product of either force by the distance between the lines of action 
of the forces. 



30 MECHANICS 

THEOREM. Two couples having the same moment and sense are 
equivalent. 

Suppose first that the forces of the one couple are parallel to the 
forces of the other couple. Then, by proper choice of the axis 
of x, we can represent the couples as indicated, where 

J P. + P.-O. 0<P,; 

P.I , I l . P 3 + P 4 = 0, 0<P 3 ; 



p *\ " P, x^xt + h, 0<h; 

Fxo.36 J *4 = * 3 + J, < l > 

Now consider the system of four forces, P lf P 2 , P 3t P 4 . 
These are in equilibrium. For, 

P, + P 2 - P 3 - P 4 = 
and 

Pr _|_p-r _ P ,. _ /:> /r 
1 ^l I * 2 ** / 2 * 3 "^S * 4 ** / 4 

(P -4- P W P It (P -\- P } r 4- P 7 = fl 

^JTj -f X 2 / ^2 -I i V.^3 I -* 4/ *'4 ' ^3 ^ VJ> 

Hence the first couple is balanced by the negative of the second 
couple, and thus the theorem is proved for the case that all the 
forces are parallel. 

If the forces of the two couples are oblique to each other, let 
OA and OB be two lines at right angles to the forces of the first 
couple and to those of the second 
couple respectively. Lay off t wo equal 
distances, OA = h and OB = h, on 
these lines. Then by the theorem just 
proved the first couple can be repre- 
sented as indicated by the forces P 
and P.* Furthermore, the second 
couple, reversed in sense, can be rep- 
resented by the forces Q and Q. Let 

the lines of action of P at A and Q at B meet in C, and carry 
these forces forward so that each acts at C. Then the four 

* It might seem that there are two cases to be considered, for cannot the vectors 
that represent the forces of the first couple be opposite in sense? True. But 
then we can begin with the second couple. Its forces will be represented by the 
Q and Q of the diagram ; and the forces of the first couple, reversed in sense, will 
now appear as P and P. 




STATICS OF A RIGID BODY 



31 



A:(i,o) 



forces obviously are in equilibrium, for all four are equal in magni- 
tude, since by hypothesis the moments of the two given couples 
are equal ; and the forces make equal angles with the indefinite 
line OC, in such a manner that the resultant of one pair is equal 
and opposite to that of the other pair, the lines of action of these 
resultants coinciding. 

To sum up, then, the effect of a couple in a given plane is the 
same, no matter whore its forces act, and no matter how large or 
small the forces may be, provided only that the moment of the 
couple is preserved both in magnitude and in sense. 

Composition of Couples. From the foregoing it appears that two 
couples in a plane can be compounded into a single couple, whose 
moment is the sum of the moments 
of the constituent couples ; all mo- 
ments being taken algebraically. 
For, assume a system of Cartesian 
axes in the plane, and mark the 
point A : (1,0). The first couple 
can be realized by a force P 1 at A 
parallel to the axis of y (and either 
positive or negative) and an equal 

and opposite force Pi at the w 

origin, acting along the axis of y. 

The moment of this couple, taken algebraically, is obviously P,. 

Dealing with the second couple in a similar manner, we now 
have as the result two forces, P 1 and P 2 , at A parallel to the axis 
of y', and two equal and opposite forces at along the axis of 
y. These forces constitute a resultant couple, whose moment is 
the sum of the moments of the given couple. 

This last statement is at fault in one particular. It may happen 
that the second couple is equal and opposite to the first, and then 
the resultant forces both vanish. In order that this case may not 
cause an exception, we extend the notion of couple to include a 
nil couple : i.e. a couple whose forces are both zero, or whose forces 
lie in the same straight line ; and we define its moment to be 0. 
We are thus led to the following theorem. 

THEOREM. // n couples act in a plane, their combined effect is 
equivalent to a single couple, whose moment is the sum of the moments 
of the given couples. 



32 MECHANICS 

Remark. The moment of a couple is equal to the sum of the 
moments of its forces about an arbitrary point of the plane. This 
is seen directly geometrically from the definition of a moment. In 
particular, let a point be chosen at pleasure. The couple can 
be realized by two forces, one of which passes through 0. The 
moment of the couple is then equal to the moment of the other 
force about 0. 

6. Resultant of Forces in a Plane. Equilibrium. Let any 

forces act in a plane. Then they are equivalent f) to a single 
force, or ii) to a single couple ; or, finally, Hi) they are in equi- 
librium. Let be an arbitrary point of the plane. Beginning 
with the force F D let us introduce at two 
forces equal and opposite to Fj. The two forces 
checked form a couple, and the remaining 
* force is the original force F x , transferred to 




the point 0. 

Proceeding in this manner with each of the 
, ' remaining forces, F 2 , , F n , we arrive at 

a new system of forces and couples equiv- 
alent to the original system of forces and consisting of those n 
forces, all acting at 0, plus n couples. . These n forces are equiva- 
lent to a single force, R, at 0; or are in equilibrium. And the 
n couples are equivalent to a single couple, or are in equilibrium. 
In general, the resultant force, R, will not vanish, nor will the 
resultant couple disappear. The latter can, in particular, be 
realized as a force equal and opposite to R and acting at 0, and a 
second force equal to R, but having a different line of action. 
Thus the resultant of all n forces is here a single force. Inciden- 
tally we have shown that a non-vanishing couple can not be 
balanced by a non- vanishing force ; for, the effect of such a force 
and such a couple is a force equal to the given force, but trans- 
ferred to a new line of action, parallel to the old line. 

It may happen that the resultant force vanishes, but the result- 
ant couple does not. For equilibrium, it is necessary and suffi- 
cient that both the resultant force and the resultant couple vanish. 
This condition can, with the help of the Remark at the close of 
5, be expressed in the following form. 

EQUILIBRIUM. A system of n forces in a plane will be in equi- 
librium if, and only if 



STATICS OF A RIGID BODY 



33 



i) they are such as would keep a particle at rest if they all acted at 
a point; and 

ii) the sum of the moments of the forces about a point (one point 
is enoughj and it may be chosen anywhere) of the plane is zero. 

Analytically, the condition can be formulated as follows. Let 
the point about which moments are to be taken, be chosen as 
the origin, and let the force F r act at the point (x r , y r ). Then 



X r = 0, 



r=l 



2) (XrYr- yrXr) = 0. 




FIG. 40 



Example. A ladder rests against a wall, the coefficient of 
friction for both ladder and wall being the same, M- If the ladder 
is just on the point of slipping when inclined at 
an angle of 60 with the horizontal, what is the 
value of ju ? 

Since all the friction is called into play, the 
forces are as indicated in the figure, R and S being 
unknown, and JJL also unknown. 

Condition ?) tells us that the sum of the verti- 
cal components upward must equal the sum of the 
vertical components downward, or 

R + S = W. 

Furthermore, the sum of the horizontal components to the right 
must equal the sum of the horizontal components to the left, or 

S = nR. 

Finally, the moments about a point, 0, of the plane must 
balance. It is convenient to choose as a point through which a 
number of unknown forces pass; for example, one end of the 
ladder, say the upper end. Thus 

2a cos 60 R = 2a sin 60 R + a cos 60 TF, 
or 

R =V3/ 
Hence 

W 



2(1- 



S 



2 (1 - M V3) 



34 MECHANICS 

We can now eliminate R and S. The resulting equation is 



Thus 

/i = 2-V3 = 0.27. 

The other root, being negative, has no physical meaning. 

EXERCISES 

1. If in the example just discussed the wall is smooth, but the 
floor is rough, and if /* = , find all positions of equilibrium. 

2. If in the example of the text /* could be as great as 1, show 
that all positions would be positions of equilibrium. 

3. A ladder 12 ft. long and weighing 30 Ibs. rests at an angle 
of 60 with the horizontal against a smooth wall, the floor being 
rough, /u = . A man weighing 160 Ibs. goes up the ladder. How 
far will he get before the ladder slips? 

4. In the last question, how rough must the floor be to enable 
the man to reach the top? 

6. Show that a necessary and sufficient condition for equilibrium 
is that the sum of the moments about each of three points, A, B, 
and C, not lying in a line, shall vanish for each point separately. 

7. Couples in Space. THEOREM I. A couple may be transferred 
to a parallel plane without altering its effect } provided merely that its 
moment and sense are preserved. 

It is sufficient to consider two couples in parallel planes, whose 
moments are equal and opposite, and to show that their forces are 

in equilibrium. Construct a cube 
with two of its faces in the planes 
of. the couples. Then one couple can 
be represented by the forces marked 
P and Pj and the reversed couple, 
by the forces Q and Q (P = Q). 

Consider the resultant of P at 
A and Q at B. It is a force of 
p + Q (= 2P) parallel to P and 
having the same sense, and passing 
through the centre, 0, of the cube. Turn next to P at C and 
Q at D. The resultant of these forces is obviously equal and 





STATICS OF A RIGID BODY 35 

opposite to the resultant just considered and having the same 
line of action. The four forces are, then, in equilibrium. This 
completes the proof. 

Example. In a certain type of auto (Buick 45-6-23) the last bolt 
in the engine head was so near the cowl that a flat wrench could 
not be used. The garage man immediately bent a flat 
wrench through a right angle, applied one end of the 
wrench to the nut and, passing a screw driver through 
the opening in the other end, turned the nut. Thus the 
applied couple was transferred from the horizontal 
plane through the screw driver to the plane of the riut. IQ ' 

Vector Representation of Couples. A couple can be represented 
by a vector as follows. Construct a vector perpendicular to the 
plane of the couple and of length equal to the moment of the 
couple. As regards the sense of the vector, either convention is 
permissible. Let us think of ourselves as standing upright on the 
plane of the couple and looking down on the plane. If we are 
on the proper side of the plane, we shall see the couple tending to 
produce rotation in the clock-wise sense. And now the direction 
from our feet to our head may be taken as the positive sense of 
the vector or, equally well, the opposite direction. 

THEOREM II. The combined effect of two couples is the same as 
that of a single couple represented by the vector obtained by adding 
geometrically the two vectors which represent respectively the given 
couples. 

The theorem has already been proved for the case that the 
planes of the given couples are parallel or coincident. If they 

intersect, lay off a line seg- 
ment of unit length, AB, 
on their line of intersection, 
and take the forces of the 
couples so that they act at 

FlQ 43 A and B perpendicularly to 

the line AB. Then it is 
easily seen that the resultant of the two forces at A and the result- 
ant of the two forces at B form a new couple. 

Finally, the vector representations of these three couples are 
three vectors perpendicular respectively to the three planes of 
the couples, equal in length to the forces of the couples, and so 




\ R 
QX^/ 



36 MECHANICS 

oriented as to give the same figure yielded by three of the forces, 
properly chosen, only turned through 90. 

8. Resultant of Forces in Space. Equilibrium. Let any n 
forces act on a body in space. Let them be represented by the 
vectors F,, , F n . Let be an arbitrary point of space. Intro- 
duce at two forces that are equal and opposite to the force F k . 
Then the n forces F lf , F n at have a resultant : 

(1) R = F! + + F n , 

acting at 0, or are in equilibrium. And the remaining forces, 
combined suitably in pairs, yield n couples, C lt , C n , whose 
resultant couple, C, is : 

(2) C = C, + - - - + C n , 

or, in particular, vanishes ; the couples being then in equilibrium. 
In general, neither R nor C will vanish. Thus the n given forces 
reduce to a force and a couple. The plane of the resultant couple, 
C, will in general be oblique to the line of action of the resultant 
force, and hence the vector C oblique to the vector R. Let 

C = C, + C 2 , 

where C^ is collinear with R, and C 2 is perpendicular to R. The 
couple represented by C 2 can be realized by two forces in a plane 
containing the resultant force, R ; and its forces can be combined 
with R, thus yielding a single force R, whose line of action, how- 
ever, has been displaced. This leaves only the couple Cj. We 
have, therefore, obtained the following theorem. 

THEOREM. Any system of forces in space is in general equiva- 
lent to a single force whose line of action is uniquely determined, 
and to a single couple, whose plane is perpendicular to the line of 
action of the resultant force. 

In particular, the resultant force may vanish, or the resultant couple 
may vanish, or both may vanish. 

Equilibrium. The given forces are said to be in equilibrium if 
and only if both the resultant force and the resultant couple 
vanish. 

For completeness it is necessary to show that the resultant 
force, R, together with its line of action, and the resultant couple, 
C t , are uniquely determined. For it is conceivable that a differ- 



STATICS OF A RIGID BODY 



37 



ent choice, O', of the point O might have led to a different result. 
Now, the vector R is uniquely determined by (1), and so is the 
same in each case ; but C depends on the choice of 0', and so C l 
might conceivably be different from CJ, though each would be 
collinear with R. This is, however, not the case. For, reverse R 
in the second case, and also the couple C[. Then the reversed 
force and couple must balance the first force and couple. But 
this situation leads to a contradiction, as the reader will at once 
perceive. 

9. Moment of a Vector. Couples. Given a force, F, acting 
along a line //, and any point in space. By the vector moment 
of F with respect to (or about) is meant the vector 
product * /\F 

(1) M - r X F, 

where r is a vector drawn from to a point of L. 

It is a vector at right angles to the plane of and 

L, and its length is numerically equal to the 

moment of F about in that plane. Its sense 

depends on whether we are using a right-handed or a left-handed 

system. Referred to Cartesian axes 




FIG. 44 



(2) 



(3) 



M = 



x a y b z c 
X Y Z 

L = (y-V)Z- (z-e)Y 

M = (z -c)X - (x- a)Z 
N = (x-a)Y - (y- 



P:(x,y,z) 




r = r' - rj, 
r' = x i + y j + z k, 



FIG. 45 



* The student should read 3 of Appendix A. This, together with the mere 
definitions that have gone before, is all of Vector Analysis which he will need for 
the present. 



38 MECHANICS 

Vector Representation of a Couple. Let a couple consist of two 
forces, F! and F 2 : 

F, + F 2 = 0, 

acting respectively along two lines L and L 2 . The vector C 
which represents the couple is seen from the definition of the 
vector product to be : 

(4) C = r X P lf 

where r represents any vector drawn from a point of L 2 to a point 
of Lj. Let be any point of space. Then the sum of the vector 
moments of F x and F 2 with respect to yields the vector couple : 

(5) C = r, X P! + r 2 X F 2 , 

where r^ r 2 are any vectors drawn from to L 1 and L 2 respec- 
tively. For 

hence 

r X F! = T! X F! - r 2 X Fj = T! X Fj + r 2 X F 2 . 

10. Vector Representation of Resultant Force and Couple. 
Resultant Axis. Wrench. Let Pi, , F n be any system of 
forces in space. Let P be any point of space, and let equal and 
opposite forces, F* and F A , k = 1, , n, be applied at P. 
Consider the n forces F^ - - , F n which act at P. Their re- 
sultant is 

R = F! + - + F n . 

The remaining forces yield n couples, consisting each of F* at 
PA', (%k, Vk, Zk) and F& at P: (x, y, z). Let r k , r be the vec- 
tors drawn from the origin of coordinates (chosen arbitrarily) to 
P k and P respectively. Then the Jfc-th couple, C*, is represented 

by the equation : 

C* = r* X F* - r X F*. 

We are thus led to the following theorem. 

THEOREM. The given forces F lf , F n are equivalent to a single 
force, 

(6) R = F, + + F n , 

acting at P; and to a couple, 

(7) C = 5) r* X F* - r X R. 

fc-i 



STATICS OF A RIGID BODY 



39 



Resultant Axis. The resultant axis is the locus of points P, 
for which C lies along R ; i.e. is collinear with R. The condition 
for this is obviously the vanishing of the vector product : 

(8) R X C = 0, R * 0. 
Let 

(9) iXF^Li 



(10) 
Thus 

(11) L = 



R = 



Fj + Zk. 



Then the condition (8) becomes, by virtue of (7) : 

R X (Li + M j + tf k) = R X (r X R), 



i 


j 


k 




i J k 


X 


Y 


Z 


= 


X Y Z 


yZ-zY 


zX-xZ 


xY-yX 




L M N 



or: 



(12) 



This is the equation of the resultant axis in vector form. To 
reduce to ordinary Cartesian form, equate the coefficients of i, j, 
k respectively. Thus we find : 

Y + zZ = YN - ZM 



(13) 



- Z (xX 



zZ) = ZL - XN 

zZ) = XM - YL 



One of these equations may become illusory through the vanish- 
ing of all the coefficients ; but some two always define intersecting 
planes, for the rank of the determinant is 2, since R > ; and 
between the three equations there exists an identical relation. 

Let ( , ij, f ) be the coordinates of the nearest point of the line to 
the origin. Then 



Hence 
(15) $ 



YN -ZM 



>? = 



ZL-XN 



ZM- YL 
ft 2 



40 MECHANICS 

Thus we have found one point of tt*e resultant axis, and the 
direction of the axis is that of R. The resultant couple is given 
by (7), where 
(16) r = i + Tjj + fk. 

Wrench. A wrench is defined as two forces, acting at arbitrary 
points; moreover, neither force shall vanish, and their lines of 
action shall be skew. 

Let the forces be F*, acting at (xk, y^ Zk), k = 1, 2. The reader 
will do well to compute the resultant force, axis, and couple. 
Suppose, in particular, that F x is a unit force along the positive 
axis of Z, and F 2 is a force of 2, parallel to the axis of y and acting 
at the point (1, 0, 0). 

EXERCISE 

Let F! and F 2 be two forces, the sum of whose moments about 
a point is 0. Show that F t , F 2 , and lie in a plane. 

11. Moment of a Vector about a Line. Let a line, L, and a 
vector, F, be given. Let L' be the line of F, and let 0, O f be the 
points of L and L' nearest together. Let r be the vector from 

to 0', and let | r | = h. Let a be 
a unit vector along L. Assume co- 
z ordinate axes as shown. Then 



r L^r By the moment of F about L is meant : 

FlG - 46 M = hY a, 

where a = k. The moment M can be expressed in invariant 
form as follows. Since 

r = hi, 
we have : 

r X F =- 



k (r X F) = hY. 
Hence 

(1) M = {a-(rXF))a. 

More generally, r may be any vector drawn from a point of L 
to a point of L'. We have thus arrived at the following result. 



STATICS OF A RIGID BODY 41 

The moment of a vector F about a line L is given by the formula : 
M = {a- (r X F)}a, 

where r is any vector drawn from a point of L to a point of the line 
of F, and a is a unit vector collinear with L and having the sign 
attributed to L. 

In particular, the moments of F about the three axes are re- 
spectively : 

yZ - zY, zX - xZ, xY - yX. 

EXERCISE 

A force of 12 kgs. acts at the point ( 1, 3, 2), and its direc- 
tion cosines arc (3, 4, 12). Find its moment about the 
principal diagonal of the unit cube; i.e. the line through the 
origin, making equal angles with the positive axes. 

12. Equilibrium. In 8 we havo obtained a necessary and 
sufficient condition for the equilibrium of n forces, F,, , F n , 
in terms of the vanishing of the resultant force and the resultant 
couple. By means of Equations (6) and (7) of 10 we can formu- 
late these conditions analytically. The first, namely, R = 0, 
gives : 



and now the second, namely, C = 0, reduces Equation (7) to the 
vanishing of the first term on the right, or 

(2) 2 (y k Z k - z k Y k ) =0, 2 (z k X k - x k Z k ) = 0, 



This last condition, which was obtained from the vanishing of 
a couple, admits two further interpretations in terms of the 
vanishing of vector moments, namely : 

i) The sum of the vector moments of the given forces with 
respect to an arbitrary point of space is 0. 

ii) The sum of the vector moments of the given forces about 
an arbitrary line of space is 0. 

The condition ii) is equivalent to the following : 

ii f ) The sum of the vector moments of the given forces about 
each of three particular non-complanar lines is 0. 



42 MECHANICS 

Necessary and Sufficient Conditions. It is important for clear- 
ness to analyse these conditions further, as to whether they are 
necessary or sufficient or both. 

Condition i), regarded as a necessary condition, is broadest when 
is taken as any point of space. But Condition ii) is sufficient 
if it holds for the lines through just one particular point 0, the 
condition (1) being fulfilled. 

Condition ii), regarded as a necessary condition, is broadest 
when the line is taken as any line in space. But as a sufficient 
condition, though true as formulated, it is less general than 
(1) and Condition ii'), which may, therefore, be taken as the 
broadest formulation of the sufficient condition. 

EXERCISES 

1. Show that Condition i) is sufficient for equilibrium. 

2. Show that Condition ii) is sufficient for equilibrium. 

13. Centre of Gravity of n Particles. Let the n particles 
^i, , w n be acted on by gravity. Thus n parallel forces arise, 
and since they have the same sense, they have a resultant not 0. 

Let the axis of z be vertical and directed downward. Then 
the resultant is a force directed downward and of magnitude 

n 

(1) R = Wj g + + m n g = g 5) m k , 



the resultant axis being vertical. Furthermore, Xk = 0, Y k = 0, 
Z k = m k g. Thus, 10, (11): 

n n 

(2) L = g V m k yk, M = - g V m k x k , N = 0. 

t-l *-i 

The nearest point of the resultant axis to the origin has the coordi- 
nates given by (15), 10 : 

(3) * = *=5-, .,_**> .-f-0. 



If any point of this line is sustained, the system of particles 
(thought of as rigidly connected) will be supported, and the 
system will remain at rest. In particular, one point on this line 
has the coordinates : 



STATICS OF A RIGID BODY 43 

If, secondly, we allow gravity to act parallel to the axis of x, 
the resultant axis now becomes parallel to that axis, and the nearest 
point to the origin is found by advancing the letters cyclically 
in Equations (3). Again the point whose coordinates are given 
by (4) lies on this axis. And, similarly, when gravity acts parallel 
to the axis of y. It seems plausible, then, that if this point be 
supported, the system will be at rest, no matter in what direction 
gravity acts. This is, in fact, the case. To prove the statement, 
let the point P of 10 be taken as (x, y, 0). Then C = 0. For 






m k a m k p m k y 



i j k 

X ij 2 

S nik y 



since the coefficient of each of the unit vectors i, j, k is seen at 
once to vanish, no matter what values a, 0, 7 may have. 

Thus the existence of a centre of gravity for n particles is 
established. It is a point such that, no matter how the system 
be oriented, the resultant couple due to gravity is nil. 

14. Three Forces. If three non-vanishing forces, acting on 
a rigid body, are in equilibrium, they lie in a plane and either pass 
through a point or are parallel. 

Proof. If two forces in space are in equilibrium, they must be 
equal and opposite, and have the same line of action ; or else each 
must vanish. Exclude the latter case as trivial. Take vector 
moments about an arbitrary point, O, in the line of action of one 
of the forces. Then the vector moment of the other force must 
vanish by 12. Thus the second force either vanishes or passes 
through ; i.e. through every point of the line of action of the 
first force. Finally, they must be equal arid opposite. 

In the case of three forces, no one of which vanishes, and no 
two of which have the same line of action, take vector moments 
about a point in the line of action of the first force, but of no 
other force. The sum of the second and third vector moments 
about must be zero. Hence the second and third forces lie in 
a plane through 0. They are, therefore, equivalent to a single 
force a couple is impossible, since it could not be balanced by the 
first force. Thus the first force reduces to the resultant, reversed 
in sense, of the second and third forces, and the theorem is proved. 



44 



MECHANICS 



A Trigonometric Theorem. The following trigonometric theorem 
is useful in many problems of the equilibrium of a body acted on 
by three forces. Let a line be drawn from the vertex of a triangle, 
dividing the opposite side into two segments of lengths m and n, 
and making angles 6 and <p with these sides. Then 

(m + n) cot if/ m cot 6 n cot <p, 

where \l/ is the angle this line makes with the 
segment n. 

The proof is immediate. Project the sides 
of the triangle on this line, produced : 

(m + n) cos \(/ = a cos 6 cos <p t 
and then apply the law of sines : 

m b n 




FIG. 47 





sin i 



sin0' 



sn 



sn <p 




Example 1. A uniform rod of length 2a is held by a string 
of length 21 attached to one end of the rod arid to a peg in a 
smooth vertical wall, the other end of the rod 
resting against the wall. Find all the positions 
of equilibrium. 

The three forces of W, T, and R must pass 
through a point, and this must be the mid-point 
of the string. Hence, applying the above trigo- 
nometric theorem to either of the triangles ABO 
or ABC, we have : 

(1) 2 tan 6 = tan <p. 

A second relation is obtained from purely geometrical consider- 
ations, namely : * 

(2) I cos = 2a cos <p. 

It remains to solve these equations. Squaring (1) and reducing, 

we have : 

4 sec 2 6 = 3 + sec 2 <p, 
or: 

4 cos 2 <p 



cos 2 = 



1+3 cos 2 <p 



* It would be possible to use the geometric relation 

/ sin = a sin <p. 
But the further computation of the solution would be less simple. 



STATICS OF A RIGID BODY 45 



Combining with (2), we get 

4Z 2 cos 2 <p 



= 4a 2 cos 2 t 



1 + 3 cos 2 <p 
Since cos <p cannot vanish, it follows that 



cos <p = 



But a and I are not unrestricted, for < cos ? < 1. Hence 



and so a < I < 2a, 

or, the string must be longer than the rod, but not twice as long. 
Furthermore, there are always two positions of equilibrium, in 
which the rod is vertical, regardless of I and a. 

Remark. What the trigonometric theorem has done for us is 
to eliminate the forces. Without it, we should have been obliged 
to write down two or three equations involving T and R, and then 
eliminate these unknowns, with which we have no concern so 
far as the position of equilibrium goes. 

Example 2. Suppose that, in the last example, the wall is 
rough. Then there is, in addition, an upward force of friction, 
F /xft, making four forces in all, when the rod is just on 
the point of slipping down the wall. But the 
forces R and F can be compounded into a single 
force S making an angle \ with the normal to 
the wall, and so the problem is reduced to a 
three-force problem. Applying the trigonometric 
theorem to the triangle ABC we find : 

2a cot <p = a cot 6 a tan \, 

(3) 2 cot <p = cot - /z. 

It is better here to take the geometric relation in the form : 

(4) I sin 8 = a sin (p. 
From (3) we now have : 

esc 2 = 4 cot 2 <p + 4/i cot <p + M 2 + 1. 




Hence 



72 

Z 2 sin 2 = - A - - : : - : - ; r-rr = 2 sin 2 
4 cot 2 99 + 4/i cot <p + M 2 + 1 



46 



MECHANICS 



This last equation can be given the form : 

Z 2 
4 cos 2 <p + 4/i cos <p sin <p + (1 + /j 2 ) sin 2 <p = 

This equation, in turn, could be reduced to a quartic in sin <p 
or cos <p ; but such procedure would be bad technique. Rather, 
let 

2 cos 2 <p = 1 + cos 2y?, 2 cos <p sin v? = sin 2<p, 

2 sin 2 p = 1 cos 2<p. 
The equation is thus reduced to an equation of the form : 

A cos 2<p + B sin 2^ = C, 
and now can be solved by the method of Chapter I, 6. 

EXERCISE 

1. Complete the study of Example 2, i) computing A, B, C, 
and ii) finding when the rod is just on the point of slipping up. 

(K2 
- J - 5 - M 2 ; 

ii) the same equation with the sign of M reversed. 

2. If a = 1, I = If, p, = 0.1, find all positions of equilibrium. 

EXERCISES ON CHAPTER II* 

1. Show that, in a tackle and fall which has n pulleys in each 
block, the power, P, exerted is 2n + 1 times 
the tension in the rope. 

2. What force applied horizontally to the 
hub of a wheel (at rest) will just cause the wheel 
to surmount an obstacle of height h? 

3. Two heavy beads of the same weight can 
slide on a rough horizontal rod. To the bead 
is attached a string that carries a smooth heavy 
bead. How far apart can the beads on the 
rod be placed if they are to remain at rest when 

FIG. 50 released ? 

4. A gate is raised on its hinges and does not fall back. How 
rough are the hinges? 




* Begin each problem by drawing a figure showing the forces, and the lengths 
and angles which enter. 



STATICS OF A RIGID BODY 47 

5. There has been a light fall of snow on the gate. A cat 
weighing 5 Ibs. walks along the top of the gate, and the gate 
drops. The disconcerted cat springs off. It is observed from 
her tracks in the snow that she reached a point 2 ft. from the 
end of the gate. The distance between the hinges is 2^- ft., 
and the centre of gravity of the gate is 5 ft. from the vertical 
line through the hinges. If the gate weighs 100 Ibs., what is 
the value of /z? 

6. A rod rests in a smooth hemispherical bowl, one end inside 
the bowl and the rim of the bowl in contact with the rod. Find 

the position of equilibrium. a -f V32r 2 + a 2 

Ans. cos 6 = , 

or 

where the radius of the bowl is r, the distance of the centre 
of gravity of the rod from its lower end is a, and the inclina- 
tion of the rod to the horizon, 0, provided a < 2r. 

7. A uniform rod rests with one end on a rough floor and the 
other end on a smooth plane inclined to the horizon at an angle a. 
Find all positions of equilibrium. 

8. The same problem where both floor and plane are rough. 

9. A picture hangs on a wall. Formulate the problem of 
equilibrium when the wall is smooth, and solve it. 

10. The same question where the wall is rough. 

11. A smooth rod rests with one end against a vertical wall, 
a peg distant h from the wall supporting the rod. Find the 

position of equilibrium. [ft 

Ans. cos = \ 
* a 

12. The same problem where the wall is rough, the peg being 
smooth. Find all positions of equilibrium. 

13. A barrel is lying on its side. A board is laid on the barrel, 
with its lower end resting on the floor. Find all positions of 
equilibrium. (Barrel, floor, and board are all rough.) 

14. A plank 8 ft. long is stood up against a carpenter's work- 
bench, which is 2 ft. 8 in. high. The coefficient of friction between 
either the floor or the bench and the plank is . If the plank 
makes an angle of 15 with the vertical, will it slip down when 
let go? 



48 MECHANICS 

15. A smooth uniform rod rests in a test-tube. Find the 
position of equilibrium. 

Ans. The solution is given by the equations : 

2 tan = cot ^>, r sin ^ + r = 2a cos 0. 

16. A uniform rod 2 ft. long rests with one end on a rough 
table. To the other end of the rod is attached a string 1 ft. long, 
made fast to a peg 2 ft. above the table. Find all positions of 
equilibrium. 

Ans. One system of limiting positions is given for ju = 2 
by the equations : 

cot <p = 2 + 2 cot 0, 2 cos 6 + cos <p = 2. 

Solve these equations by means of the Method of Successive 
Approximations. 

17. A water tower is 100 ft. high and 100 ft. in diameter. Find 
approximately the tension in the plates near the base. 

18. Water is gradually poured into a tumbler. Show that the 
centre of gravity of the glass and the water is lowest when it is in 
the surface of the water. 

19. If one attempts to pull out a two-handled drawer by one 
handle, what is the condition that the drawer will stick fast ? 



CHAPTER III 
MOTION OF A PARTICLE 

1. Rectilinear Motion.* Tube simplest case of motion of mat- 
ter under the action of force isHhat in which a rigid body moves 
without rotation, each point of the body describing a right line, 
and the forces that act being resolved along that line. Consider, 
for example, a train of cars, and neglect the rotation of the wheels 
and axles. The train is moved by the draw-bar pull of the loco- 
motive, and the motion is resisted by the friction of the tracks 
and the wind pressure. Obviously, it is only the components of 
the forces parallel to the tracks that count, and the problem of 
Dynamics, or Kinetics, as it is more specifically called, is to 
determine the relation between the forces and the motion; or, 
if one will: Given the forces, to find the distance traversed 
as a function of the time. 

A more conventional example, coming nearer to possible experi- 
mentation in the laboratory, would be that of a block of iron 

* The student must not feel obliged to finish this chapter before going on. What 
is needed is a thorough drill in the treatment of the early problems by the present 
methods, for these are the general methods of Mechanics, to inculcate which is 
a prime object of this book. Elementary text-books in Physics sometimes write 
down three equations : 

* = ^at 2 , v at, t? 2 = 2as, 

and give an unconscionable number of problems to be solved by this device. The 
pedagogy of this procedure is totally wrong, since it replaces ideas by a rule of 
thumb, and even this rule is badly chosen, since it disguises, instead of revealing, 
the mechanical intuition. Now, a feeling for Mechanics is the great object to 
be obtained, and the habits of thought which promote such intuition are, fortu- 
nately, cultivated by just the same mathematical treatment which applies in the 
more advanced parts of Mechanics. It is a happy circumstance that here there 
is no conflict, but the closest union, between the physics of the subject and the 
mathematical analysis. 

A thorough study of 1-12 through working each problem by the present general 
methods is most important. Moreover, 22 should here be included with, of 
course, the definition of vector acceleration given in 16 and the statement of 
Newton's Second Law in 17. The student should then turn to Chapter IV, the 
most revealing chapter in the whole elementary part of the book, and study it ic 
all detail. The remaining sections of the present chapter should be read casually 
at an early stage, so as not to impede progress. Ultimately, they are important ; 
but they are most useful when the student comes to recognize their importance 
through his experience gathered from the later work above referred to. 

49 



50 MECHANICS 

placed on a table and drawn along by cords, so applied that the 
block does not rotate and that each point of it describes a right 
line with varying velocity. 

It is clear that a block of platinum having the same mass, 
i.e. containing the same amount of matter, if acted on by the 
same forces, would move just like the block of iron, if the two were 
started side by side from rest or with the same initial velocities. 
We can conceive physical substances of still greater density, and 
the same would be true. On compressing the given amount of 
matter into smaller and ever smaller volume, we are led to the 
idea of a particle, or material point, i.e. a geometrical point, to 
which the property of mass is attached. This conception has 
the advantage that such a particle would move exactly as the 
actual body does if acted on by the same forces; but we need 
say nothing about rotation, since this idea does not enter when 
we consider only particles. Moreover, there is no doubt about 
where the forces are applied they must be applied at the one 
point, the particle. 

2. Newton's Laws of Motion. Sir Isaac Newton (1642-1727), 
who was one of the chief founders of the Calculus, stated three 
laws governing the motion of a body. 

FIRST LAW. A body at rest remains at rest and a body in motion 
moves in a straight line with unchanging velocity, unless some external 
force acts on it. 

SECOND LAW. The rate of change of the momentum of a body 
is proportional to the resultant external force that acts on the body. 

THIRD LAW. Action and reaction are equal and opposite. 

The meaning of the First Law is clear enough, if we restrict 
ourselves for the present to bodies and particles as described and 
moving in 1.* The Third Law, too, is self-explanatory. Con- 
sider, for example, two particles of unequal mass, connected by 
a spring, the mass of which is negligible. Then the pull (or push) 
of the spring on the one particle is equal and opposite to its pull 
(or push) on the other particle. 

The Second Law is expressed in terms of momentum, and the 
momentum of a particle is defined as the product of its mass by 

*We might consider, furthermore, such material distributions as laminae, i.e. 
material surfaces; and also wires, or material curves. Finally, rigid combinations 
of all these bodies. 



MOTION OF A PARTICLE 51 

its velocity, or mv. Here, v is not an essentially positive quan- 
tity the mere speed. We must think of the position of the 
body as described by a suitable coordinate, s. The latter may 
be the distance actually traversed by the particle; or we may 
think of the path of the particle as the axis of x, and s as the 
coordinate of the particle. The velocity, v, will then be defined 
as ds/dt : 



and is positive when s is increasing ; negative, when s is decreasing. 
The Second Law can now be stated in the form : 

(2) t . 



Here, / denotes the resultant force, and is positive when it tends 
to increase s ; negative, when it tends to decrease s. 

Ordinarily, m is constant always, in the case of the bodies 
cited above and so 

d (mv) _ dv 

~dT ~ m 'dt 

The quantity dv/dt is defined as the acceleration, and is often 
represented by a : 



It is positive when v is increasing, negative when v is decreasing. 
Newton's Second Law can now be stated in the form : The mass 
times the acceleration is proportional to the force : 

(4) ma oc /. 

From the proportion we now pass to an equation : 

(5) ma = X/, 

where X is a physical constant. The value of X depends on the 
units used. If these are the English units, the pound being the 
unit of mass, the foot the unit of length, the second the unit of time, 
and the pound the gravitational unit of force, then X has the 
value 32 (or, more precisely, 32.2), and Newton's Second Law of 
Motion becomes here : 

A,) m 



52 MECHANICS 

In the decimal system, the gramme being the unit of mass, the 
centimetre the unit of length, the second the unit of time, and the 
gramme the gravitational unit of force, X = 981, and Newton's 
Second Law of Motion becomes here : 

A 2 ) mf t = 981 /. 

In 3 we shall discuss the absolute units. In particular, the 
units of mass, length, and time having been chosen arbitrarily, 
as in Physics, the so-called "absolute unit of force " is that unit 
which makes X = 1 in Newton's Equation, so that here : 

A \ dv . 

A,) m di =f - 

Three Forms for the Acceleration. The acceleration is defined 
as dv/dt, and since v = ds/dt, we have : 

x/2 

/!\ U * 

(6) a = ^ 

A third form is obtained by starting with the equation : 

(7\ dv _ dsdv 

( ' dt ~ di ds 

and then replacing ds/dt by its value, v. Thus 
(8) . - .*. 

These three forms for the acceleration : 

dv d z s dv 



connect the three letters s, t, v in pairs in all possible ways. Which 
form it is better to use in a given case, will become clear from 
practice in solving problems. 
Example 1. A freight train weighing 200 tons is drawn by 

a locomotive that exerts a draw- 

jt PP-I / ==8000 t bar pull of 9 tons. 5 tons of this 

s force are expended in overcoming 

frictional resistances. How much 

speed will the train have acquired at the end of a minute, if it 
starts from rest? 



MOTION OF A PARTICLE 63 

Here we have 

m - 200 X 2000 = 400,000 Ibs., 

/ = 9 X 2000 - 5 X 2000 = 8000 Ibs.* 
and hence Equation A,) becomes : 

400,000^ = 32X8000, 

or = 

dt 25 

Integrating with respect to t, we find : 

V == Tjngt ~f~ C . 

Since v = when t = 0, we must have C 0, and hence 

At the end of a minute, t = 60, and so 

^ = M X 60 = 38 - 4 ft - P er sec. 

To reduce feet per second to miles per hour it is convenient 
to notice that 30 miles an hour is equivalent to 44 ft. a second, 
as the student can readily verify; or roughly, 2 miles an hour 
corresponds to 3 ft. a second. Hence the speed in the present 
case is about two-thirds of 38.4, or 26 miles an hour. 

Example 2. A stone is sent gliding over the ice with an initial 
velocity of 30 ft. a sec. If the coefficient of friction between the 
stone and the ice is -fa, how far will the stone go ? 

Here, the only force that we take account of is the retarding 
force of friction, and this amounts to one-tenth of a pound of force 
for every pound of mass there is m 
in the stone. Hence, if there are 4 \ 10 -q 



m pounds of mass in the stone s 

the force will be ^m lbs.,f and FlG * 52 

since it tends to decrease s, it is to be taken as negative: 



* The student must distinguish carefully between the two meanings of the word 
pound, namely (a) a mass, and (6) a force two totally different physical objects. 
Thus a pound of lead is a certain quantity of matter. If it is hung up by a string, 
the tension in the string is a pound of force. 

t The student should notice that m is neither a mass nor a force, but a number, 
like all the other letters of Algebra, the Calculus, and Physics. 



54 MECHANICS 

Now what we want is a relation between v and s, for the ques- 
tion is: How far (s = ?), when the stone stops (v = 0)? So we 
use the value (8) of a and thus obtain the equation : 

dv 16 
V ds = ~-5> 

or v dv = /-ds. 

rr " 2 16 . n 

Hence T> = ^- s + C. 

To determine C we have the data that, when s = 0, v = 30. 
Since in particular the equation must hold for these values, 

^! = + C, C = 450, 

and so v 2 = 900 - ^s. 

When the stone stops, v = 0, and we have 

= 900 - 3s, s = 141 ft. 

EXERCISES * 

1. If the train of Example 1 was moving at the rate of 4 m. 
an hour when we began to take notice, how fast would it be mov- 
ing half a minute later? Give a complete solution, beginning with 
drawing the figure. Ans. About 17 m. an h. 

2. A small boy sees a slide on the ice ahead, and runs for it. 
He reaches it with a speed of 8 miles an hour and slides 15 feet. 
How rough are his shoes? Ans. M = .15. 

3. Show that, if the coefficient of friction between a sprinter's 
shoes and the track is T V> n ^ ^ cs ^ possible record in a hundred- 
yard dash cannot be less than 1 5 seconds. 

4. An electric car weighing 12 tons gets up a speed of 15 miles 
an hour in 10 seconds. Find the average force that acts on it, 

* It is important that the student should work these exercises by the method 
set forth in th 4 e text, beginning each time by drawing a figure and marking (t) the 
force, by means of a directed right line, or vector, drawn preferably in red ink ; 
and (t'i) the coordinate used, as s or x, etc. He should not try to adapt such formulas 
of Elementary Physics as 

v = at, a = a 2 , v z = 2as 

to present purposes. For, tho object of these simple exercises is to prepare the way 
for applications in which the force ia not constant, and here the formulas just cited 
do not hold. 



MOTION OF A PARTICLE 55 

i.e. the constant force which would produce the same velocity in 
the same time. 

6. In the preceding problem, assume that the given speed is 
acquired after running 200 feet. Find the time required and 
the average force. 

6. A train weighing 500 tons and running at the rate of 30 miles 
an hour is brought to rest by the brakes after running 600 feet. 
While it is being stopped it passes over a bridge. Find the force 
with which the bridge pulls on its anchorage. Ans. 25.2 tons. 

7. An electric car is starting on an icy track. The wheels 
skid and it takes the car 15 seconds to get up a speed of two miles 
an hour. Compute the coefficient of friction between the wheels 
and the track. 

3. Absolute Units of Force. The units in terms of which we 
measure mass, space, time, and force arc arbitrary, as was pointed 
out in 2. If we change one of them, we thereby change the 
value of X in Newton's Second Law. Consequently, by changing 
the unit of force properly, the units of mass, space, and time being 
held fast, we can make X = 1. Hence the definition above given: 

DEFINITION. The absolute unit of force _is that unit which 
makes X = 1 in Newton's_ Second Law of Motion ij* 

(1) moT^f. 

In order to determine experimentally the absolute unit of force, 
we may allow a body to fall freely and observe how far it goes in 
a known time. It is a physical law that the force with which 
gravity attracts any body is proportional to the mass of that body. 
Let the number g be the number of absolute units of force with 

* We have already met a precisely similar question twice in the Calculus. In 
differentiating the function sin x we obtain the formula 

D x sin x = cos x 
only when we measure angles in radians. Otherwise the formula reads: 

D x sin x X cos x. 

In particular, if the unit is a degree, X = Tr/180. We may, therefore, define a radian 
as follows : The absolute unit of angle (the radian) is that unit which makes X = 1 
in the above equation. 

Again, in differentiating the logarithm, we found ; 



X 

This multiplier reduces to unity when we take a = e. Hence the definition : 
The absolute (natural) base of logarithms is that base which makes the multiplier 
logo e in the above equation equal to unity. 



56 MECHANICS 

which gravity attracts the unit of mass. Then the force, measured 
in absolute units, with which gravity attracts a body of m units 
of mass will be mg. Newton's Second Law A 3 ) gives for this case : 

dv , dv 



ds 



s = %gt* + K, K = 0, 

and we have the law for freely falling bodies deduced directly 
from Newton's Second Law of Motion, the hypothesis being 
merely that the force of gravity is constant. Substituting in 
the last equation the observed values s = S, t = T, we get : 

28 

9 = ?*' 

If we use English units for mass, space, and time, g has, to 
two significant figures, the value 32, i.e. the absolute unit of 
force in this system, a poundal, is equal nearly to half an ounce. 
If we use c.g.s. units, g ranges from 978 to 983 at different parts 
of the earth, and has in Cambridge the value 980. The absolute 
unit of force in this system is called the dyne. 

Since g is equal to the acceleration with which a body falls 
freely under the attraction of gravity, g is called the acceleration 
of gravity. But this is not our definition of g ; it is a theorem 
about g that follows from Newton's Second Law of Motion. 

The student can now readily prove the following theorem, 
which is often taken as the definition of the absolute unit of 
force in elementary physics : The absolute unit of force is that 
force which, acting on the unit of mass for the unit of time, gener- 
ates the unit of velocity. 

Incidentally we have obtained two of the equations for a freely 
falling body : 

v = gt, s = %gt 2 . 

The third is found by setting a = v dv/ds and integrating : 

dv 



2gs. 



MOTION OF A PARTICLE 



57 



Example. A body is projected down a rough inclined plane 
with an initial velocity of V Q feet per second. Determine the 
motion completely. 

The forces which act are : the component of gravity, mg sin 7 
absolute units, down the plane, and the force of friction, pR = 
nmg cos 7 up the plane. Hence 
ma = mg sin 7 nmg cos 7, 

dv 

-IT = g sm 7 



cos 7. 



Integrating this equation, we 
get 
v = g (sin 7 /z cos 7) t + C, 

o = + <?> 



= g (sin 7 - 




cos 7) + v . 



A second integration gives 

B) s = \g (sin 7 - ^ cos 7) P + V Q t, 

the constant of integration here being 0. 

To find v in terms of s we may eliminate t between A) and 
B). Or we can begin by using formula (8), 2, for the acceler- 

ation : 

dv f . , 

v-r = g (sin 7 - /x cos 7), 

do 

%v 2 = g (sin 7 M cos 7) s + K, 

^ = + X, 

t; 2 = 20 (sin 7 /z cos 7) s + #o- 

EXERCISES 

1. If, in the example discussed in the text, the body is pro- 
jected up the plane, find how far it will go up. 

2. Determine the time it takes the body in Question 1 to 
reach the highest point. 

3. Obtain the usual formulas for the motion of a body pro- 
jected vertically : 

v 2 = 2gs + vl or = 2gs + vl ; 

v = gt + V Q or = - gt + V Q ; 

8 = ot* + v t or =-tf* + M. 



58 MECHANICS 

4. On the surface of the moon a pound weighs only one-sixth 
as much as on the surface of the earth. If a mouse can jump 
up 1 foot on the surface of the earth, how high could she jump 
on the surface of the moon? Compare the time she is in the air 
in the two cases. 

6. A block of iron weighing 100 pounds rests on a smooth 
table. A cord, attached to the iron, runs over a smooth pulley 
at the edge of the table and carries a weight of 15 pounds, which 
hangs vertically. The system is released with the iron 10 feet 
from the pulley. How long will it be before the iron reaches the 
pulley, and how fast will it be moving? 

Ans. 2.19 sec. ; 9.1 ft. a sec. 

6. Solve the same problem on the assumption that the table is 
rough, n = ^, and that the pulley exerts a constant retarding 
force of 4 ounces. 

7. Regarding the big locomotive exhibited at the World's 
Fair in 1905 by the Baltimore and Ohio Railroad the Scientific 
American said : "Previous to sending the engine to St. Louis, the 
engine was tested at Schenectady, where she took a 63-car train 
weighing 3150 tons up a one-per-cent. grade." 

Find how long it would take the engine to develop a speed 
of 15 m. per h. in the same train on the level, starting from rest, 
the draw-bar pull being assumed to be the same as on the grade. 

8. If Sir Isaac Newton registered 170 pounds on a spring 
balance in an elevator at rest, and if, when the elevator was 
moving, he weighed only 169 pounds, what inference would he 
draw about the motion of the elevator? 

9. What does a man whose weight is 180 pounds weigh in an 
elevator that is descending with an acceleration of 2 feet per 
second per second ? 

4. Elastic Strings. When an elastic string is stretched by a 
moderate amount, the tension, T, in the string is proportional 
to the stretching, i.e. to the difference, s, between the stretched 
and the unstretched length of the string : 

(1) T oc s, or T = ks, 

where fc is a physical constant, whose value depends both on the 
particular string and on the units used. 



MOTION OF A PARTICLE 59 

Suppose, for example, that a string is stretched 6 in. by a force 
of 12 Ibs. ; to determine k. If we measure the force in gravitar 
tional units, i.e. pounds, then 

T = 12 when s = . 

Hence, substituting these values in equation (1), we have: 
12 = &, or k = 24, 

(2) T = 24s. 

If we had chosen to measure the force in absolute units, i.e. 
poundals, then, since it takes (nearly) 32 of these units to make 
a pound, the given force of 12 pounds would be expressed as 
(nearly) 12 X 32, or precisely 120, poundals. Hence, substitut- 
ing the present value of the force in (1), which, to avoid con- 
fusion, we will now write in the form : 

T = k's, 
we have : 120 = k' \ or k' = 240, 

(3) T' = 240s. 

When the string is stretched 1 in., s = ^ and the tension 
as given by (2) is T = 2, i.e. 2 pounds. Formula (3), on the 
other hand, gives 20, or 64 (nearly) as the value of the ten- 
sion, expressed in terms of poundals, and this is right; for it 
takes 64 half-ounces to make 2 pounds, and so we should have 
T' = 20.* 

The law of strings stated above is familiar to the student in the 
form of Hooke's Law: 

rr\ __. 



I ' 

where I is the natural, or unstretched, length of the string, and 
l f , the stretched length; the coefficient E being Young's Mod- 
ulus. For a given string, E/l = k is constant, and V I = s is 
variable. 

* It is easy to check an answer in any numerical case. The student has only 
to ask himself the question: "Have I expressed my force in pounds, or have I 
expressed it in terms of half-ounces?" Just as five dollars is expressed by the 
number 5 when we use the dollar as the unit, but by the number 500 when we 
use the cent, so, generally, the smaller the unit, the larger the number which expresses 
a given quantity. 



60 MECHANICS 

EXERCISES 

1. An clastic string is stretched 2 in. by a force of .3 Ibs. Find 
the tension (a) in pounds; (b) in poundals, when it is stretched 
s ft. Ans. (a) T = 18s ; (6) T = 180s. 

2. When the string of Question 1 is stretched 4 in., what is 
the tension (a) in terms of gravitational units; (b) in terms of 
absolute units? Ans. (a) 6 pounds; (6) 192 poundals. 

3. An elastic string is stretched 1 cm. by a force of 100 grs. 
Find the tension (a) in grs. ; (6) in dynes, when it is stretched 
s cm. Ans. (a) 100s; (b) 98,000s. 

4. One end of an elastic string 3 ft. long is fastened to a peg 
at A, and a 2-pound weight is attached to the other end. The 
weight is gradually lowered till it is just supported by the string, 
and it is found that the length of the string has thus been doubled. 
Find the tension in the string when it is stretched s ft. 

Ans. f s Ibs. ; ^s poundals. 

5. A Problem of Motion. One end of the string considered 
in the text of 4 is fastened to a peg at a point of a smooth 
horizontal table ; a weight of 3 Ibs. is attached to the other end 
of the string and released from rest on the table with the string 

.stretched one foot. How fast will the weight be moving when 
the string becomes slack? 

The weight evidently describes a straight line from the starting 
point, A, toward the peg 0, and we wish to know its velocity 
when it has reached a point B, one foot from A. 

The solution is based on Newton's Second Law of Motion. 
It is convenient here to take as the coordinate, not the distance 

AP that the particle has travelled at 

- - - < - ' - -j any instant, but its distance s from B. 
T-, KA The force which acts is the tension 

riG. 54 i.i 

of the string; measured in absolute 

units it is 240rs. Since it tends to decrease s, it is negative. 
Hence Newton's Law becomes : 

(1) 
(2) 



___ fJ2 a tit) 

To integrate this equation, replace -^ by its value v -=- : 



MOTION OF A PARTICLE 61 

Hence v dv = 



(3) 



I v dv = 8g I sds, 



To determine C, observe that initially, i.e. when the particle 
was released at A, v = and s = I. Hence 

= - 4(7 + C, C = 40, 

and (3) becomes 
(4) t; 2 = 80 (1 - s 2 ). 

We have now determined the velocity of the particle at an 
arbitrary point of its path, and thus are in a position to find its 
velocity at the one point specified in the question proposed, 
namely, at B. Here, s = 0, and 

v 2 Uo = 8g = 8 X 32, v\ s=sQ = 16 (ft. per sec.) 

EXERCISES * 

1. The weight in the problem just discussed is projected from 
B along the table in the direction of OB produced with a velocity 
of 8 ft. per sec. Find how far it will go before it begins to return. 

Ans. Newton's equation is the same as before, and the 
integral, (3), is the same ; but initially s = and v = 8. 
Hence C = 32, and the answer is 6 inches. 

2. If, in the example worked in the text, the table is rough 
and the coefficient of friction, /i, has the value ^, how fast will 
the body be moving when it reaches B ? 

Ans. Newton's equation now becomes : 

3^=-24g8 + i-3g, 

and the answer is : 4 Vl5 = 15.49 ft. per sec. 

3. Solve the problem of Question 1, for a rough table, M = T- 
Ans. The required distance is the positive root of the 

equation 16s 2 + s 4 = 0, or s = .4698 ft., or about 
5fin. 

* In the following exercises and examples, it will be convenient to take the value 
of g as exactly 32 when English units are used. Begin each exercise by drawing a 
figure showing the coordinate used, and mark the forces in red ink. 



62 MECHANICS 

4. Find where the weight in Question 2 will come to rest 
if the string, after becoming slack, does not get in the way. 

6. The 2 Ib. weight of Question 4, 4, is released from rest 
at a point B directly under the peg .4 and at a distance of 3 ft. 
from A ; the string thus being taut, but not stretched. Find 
how far it will fall before it begins to rise. Ans. 6 ft. 

6. If, in the last question, the weight is dropped from the 
peg at A, find how far it descends before it begins to rise. 

Ans. To a distance of 6 + 3\/3 = 11.196 ft. below A. 

7. If the weight in the last two questions is carried to a point 
7 ft. below A and released, show that it will rise to a distance of 
5 ft. below A before beginning to fall. 

8. If, in the last question, the weight is released from a point 
10 ft. below A, show; that it will rise to a height of 1 ft. and 10 in. 
below A. 

9. The string of the example studied in the text of 4 is 
placed on a smooth inclined plane making an angle of 30 with 
the horizon, and one end is made fast to a peg at A in the plane. 
If a weight of 1 Ibs. be attached to the other end of the string 
and released from rest at A, find how far down the plane it will 
slide. Assume the unstretched length of the string to be 4 ft. 

10. The same question if the plane is rough, /* = ^V3. 

11. A cylindrical spar buoy (specific gravity ^) is anchored 
so that it is just submerged at high water. If the cable should 
break at high tide, show that the spar would jump entirely out 
of the water. 

Assume that the buoyancy of the water is always just equal 
to the weight of water displaced. 

12. A particle of mass 2 Ibs. lies on a rough horizontal table, 
and is fastened to a post by an elastic band whose unstretched 
length is 10 inches. The coefficient of friction is -, and the band 
is doubled in length by hanging it vertically with the weight at 
its lower end. If the particle be drawn out to a distance of 
15 inches from the post and then projected directly away from 
the post with an initial velocity of 5 ft. a sec., find where it will 
stop for good. 



MOTION OF A PARTICLE 63 

6. Continuation ; the Time. The time required by the body 
whose motion was studied in 5 to reach the point B can be 
found as follows. From equation (4) we have : 

(5) v = -^ = V8g Vl s 2 . 

Since s decreases as t increases, ds/dt is negative, and the lower 
sign holds. Replacing V8g by its value, 16, we see that 

(6) 

This differential equation is readily solved by separating the 
variables, i.e. by transforming the equation so that only the 
variable s occurs on one side of the new equation, and only t on 
the other ; thus 

(7) I6dt = - 

Hence 16* = - f , ds = - sin- 1 s + C. 



= - f , ds = - si 

J Vl - s 2 



If we measure the time from the instant when the body was 
released at A, then t = arid s = 1 are the initial values which 
determine C : 

= - sin- 1 1 + C, C = ~ 

Thus l&t = - sin- 1 s. 



The right-hand side of this equation has the value cos"" a . 
Hence we have, as the final result,* 

(8) 16t = cos" 1 s, or s = cos 16$. 

* In evaluating the above integral we might equally well have used the formula 



Vl - 2 
We should then have had : 

16* = cos- 1 8 - C'. 
Substituting the initial values t - 0, * = 1 in this equation, we find : 

= cos' 1 1 - C", or C" - 0, 
and the final result is the same as before. 



64 MECHANICS 

This equation gives the time it takes the body to reach an 
arbitrary point of its path. In particular, the time from A to 
B is found by putting s = : 

(9) W = cos- 1 = |, t = J2 = .09818 sec. 

EXERCISES 

1. Show that if the body, in the case just discussed, had been 
released from rest at any other distance from the peg, the string 
being stretched, the time to the point at which the string becomes 
slack would have been the same. 

2. Show that it takes the body twice as long to cover the first 
half of its total path as it does to cover the remainder. 

Find the time required to cover the entire path in the case 
of the following exercises at the close of 5. 

3. Exercise 1. Ans. ^ = .09818. 

OA 

4. Exercise 5. 

Ans. t = \^K / / -', total time, TrA/^ = .9618 sec. 

* 04 J v 6s s 2 ^ 

5. Exercise 6. Ans. t = \ ^ + sin- 1 77= =? 

6. Exercise 7. Ans. .9618 sec. 

7. Exercise 9. 8. Exercise 10. 9. Exercise 8. 

7. Simple Harmonic Motion. The simplest and most important 
ease of oscillatory motion which occurs in nature is that known 
as Simple, Harmonic Motion. It is illustrated with the least 
amount of technical detail by the following example, or by the 
first Exercise below. 

Example. A hole is bored through the centre of the earth, a 
stone is inserted, the air is exhausted, and the stone 
is released from rest at the surface of the earth. 
To determine the motion. 

The earth is here considered as a homogeneous 
sphere, at rest in space. Its attraction, F, on 

^ the stone diminishes as the stone nears the cen- 

FIG. 55 tre, and it can be shown to be proportional, at 




MOTION OF A PARTICLE 65 

any point of the hole, to the distance of the stone from the 

centre: ~ , 

F oc r, or F = kr. 

To determine the constant fc, observe that, at the surface, 
r = R (the radius of the earth), and, if we measure F in absolute 
units, F = wgr, where m denotes the mass of the stone. Hence 

mg = kR or k = ~^, 

/ 

and F = ^r 

R 

As the coordinate of the stone we will take its distance, r, 
from the centre of the earth. Then Newton's Second Law gives 
us: 
/i\ d*r mg 

(1) m ^ = -R r - 

For, when r Ls positive, the force tends to decrease r, and so is 
negative. When r is negative, the force tends to increase r alge- 
braically, and so is positive. Hence (1) is right in all cases. 

In order to integrate Equation (1), which can be written in 
the form : 

(2) <*L=-L r 
w dp R r > 

we employ the device of multiplying through by 2dr/dt: 

cydrd^r = _ 2g dr 
dtdt*~ R T dt 

d /rfr\ 2 

The left-hand side thus becomes -77 ( -n ) Hence each side 

at \dt/ 

can be integrated with respect to t : * 

* This method can be applied to any differential equation of the form : 



Multiply through by 2 dy/dx : 

a 4? 

<&c cte 2 
The left-hand side thus becomes ( ~ J Hence 



Integrating, we have 



66 MECHANICS 

--^.Cr^ 
~ R r dt 



C d ( 
Jdt\dt 



or 

_ - - 

dt ~ R - R 

To determine (7, observe that initially, i.e. when the stone was 
at Ay r = R and the velocity, dr/dt, = 0. Hence 

0=~|ft2 + c, or C = !# 2 . 
7 it 

Thus finally : 

< 3 > (I)'- 1 <'-"> 

At the centre of the earth, r = 0, and (dr/dt) 2 = gR. If we 
take the radius of the earth as 4000 miles, then R = 4000 X 5280, 
g = 32, and the velocity is about 26,000 ft. a sec., or approxi- 
mately 5 miles a second. 

The stone keeps on with diminishing speed and comes to rest 
for an instant when r = J?, i.e. it just reaches the other side 
of the earth, and then falls back. Thus it oscillates throughout 
the whole length of the hole, reaching the surface at the end of 
each excursion, and continuing this motion forever. The result 
is not unreasonable, for there is no damping of any sort, no 
friction or air resistance. 

The Time. To find the time we proceed as in 6. From 
Equation (3) it follows that 



Hence, separating the variables, we have : 

'" dr 



dt = - \ F ====^. 
9 VR* - r 

or t = ^\| cctfh 1 ~ + C. 

I 
Initially, t = and r = 72 ; thus (7 = 0, and 

(4) t = \ cos- 1 ~, or r = R cos (^ VB) ' 

* <7 /t \ A// 



MOTION OF A PARTICLE 67 

The time from A to is found by putting r = : 

* 

-' 

On computing the value of this expression it is seen to be 21 min. 
and 16 sec. The time from A to B is twice the above. Hence 
the time of a complete excursion, from A to B and back to A is 





This time is known as the period of the oscillation.* 

The General Case. Simple Harmonic Motion is always dom- 
inated by the differential equation 

A\ ** X _ % ~ 

' ~dfi ~ ' 

where the coordinate x characterizes the displacement from the 
position of no force. This equation can be integrated as in the 
special case above, and it is found that 

B) 

where h denotes the value of x which corresponds to the extreme 
displacement. The velocity when x = is numerically nh, and 
thus is proportional both to n and to h. A second integration 
gives 

C) x = h cos ntj 

provided the time is measured from an instant when x = h. 
The period, T, is inversely proportional to n : 

^ 27T 



and the amplitude is 2h. Thus the period is independent of 
the amplitude. 

The motion represented by Equation C) is known as Simple 
Harmonic Motion. The graph of the function is obtained from 

* In the first equation (4) the principal value of the anti-cosine holds during 
the first passage of the stone from A to B. The second equation (4) holds with- 
out restriction. 



68 MECHANICS 

the graph of the cosine curve by plotting the latter to one scale 
on the axis of t, and to another scale on the axis of x. 




FIG. 56 

EXERCISES 

1. Two strings like the one described in the text of 4 are 
fastened, one end of each, to two pegs, A and B, on a smooth 
horizontal table, the distance AB being double the length of 
either string, and the other end of each string is made fast to 
a 3 Ib. weight, which is placed at 0, the mid-point of AB. Thus 
each string is taut, but not stretched. The weight being moved 
to a point C between and A and then released from rest, show 
that it oscillates with simple harmonic motion. Find the velocity 
with which it passes and the period of the oscillation. It is 
assumed that the string which is slack in no wise interferes with 
or influences the motion. 

Ans. The differential equation which dominates the motion 

d 2 x 

is ffi = 256z, where x denotes the displacement of the 
at 

3 Ib. weight ; hence the motion is simple harmonic motion. 
The required velocity is numerically 16h, where h denotes 
the maximum displacement. The period is 27T/16 = 
.3927 sec. 

2. Work the same problem for two strings like the one of 
Question 4, 4, and a 2 Ib. weight. 

3. Show that the motion of Example 7, 5, is simple harmonic 
motion, and find the period. 

4. If a straight hole were bored through the earth from Boston 
to London, a smooth tube containing a letter inserted, the air 
exhausted from the tube, and the letter released at Boston, how 
long would it take the letter to reach London? 



MOTION OF A PARTICLE 69 

6. If in the problem of Question 9, 5, the weight were re- 
leased with the string taut, but not stretched, and directed straight 
down the plane, show that the weight would execute simple 
harmonic motion. Determine the amplitude and the period. 

6. Work the problem of the text for the moon; cf. the data 
in 8. 

7. A steel wire of one square millimeter cross-section is hung 
up in Bunker Hill Monument, and a weight of 25 kilogrammes is 
fastened to the lower end of the wire and carefully brought to 
rest. The weight is then given a slight vertical displacement. 
Determine the period of the oscillation. 

Given that the force required to double the length of the wire 
is 21,000 kilogrammes, and that the length of tho wire is 210 feet. 

Ans. A little over half a second. 

8. A number of iron weights are attached to one end of a long 
round wooden spar, so that, when left to itself, the spar floats 
vertically in water. A ten-kilogramme weight having become 
accidentally detached, the spar is seen to oscillate with a period 
of 4 seconds. The radius of the spar is 10 centimetres. Find 
the sum of the weights of the spar and attached iron. Through 
what distance docs the spar oscillate ? 

Ans. (a) About 125 kilogrammes ; (6) 0.64 metre. 

8. Motion under the Attraction of Gravitation. Problem. To 
find the velocity which a stone acquires in falling to the earth 
from interstellar space. 

Assume the earth to be at rest and consider only the \ A 

force which the earth exerts. Let the stone be re- j 

leased from rest at A, and let r be its distance from 
the centre of the earth at any subsequent instant. 
Then the force, F, acting on it is, by the law of 
gravitation, inversely proportional to r : 



El A 

*-? 

Since F = mg when r = JR, the radius of the earth, 

X , r mgR* 

mq = -F^ and v = ^ 




70 MECHANICS 

Newton's Second Law of Motion here takes on the form : 

d z r _ mgR 2 
m ~dT* ~ ~7*~' 
Hence 



To integrate this equation, we employ the method of 7 and 
multiply by 2 dr/dt : 

drd 2 r 2gR 2 dr d/dr\* = 2gR*dr 

dt dt 2 r 2 dt' r di\dt) r 2 dt 

Integrating with respect to t we find : 



Initially dr/dt = and T = Z ; hence 

o.' + c, c~ 



Since dr/dt is numerically equal to the velocity, the velocity 
V at the surface of the earth is given by the equation : 



If I is very great, the last term in the parenthesis is small, and 
so, no matter how great I is, V can never quite equal V2gR. 
Here g = 32, R = 4000 X 5280, and hence the velocity in ques- 
tion is about 36,000 feet, or 7 miles, a second. 

This solution neglects the retarding effect of the atmosphere; 
but as the atmosphere is very rare at a height of 50 miles from 
the earth's surface, the result is reliable down to a point com- 
paratively near the earth. 

In qrder to find the time it would take the stone to fall, con- 
sider the equation derived from (2) : 




Hence 

2 



, 
and 



MOTION OF A PARTICLE 71 

Vl r rdr 



Turning to Peirce's Tables, No. 169, we find : 

dr 



Vlr - r 2 



= V lr - r 2 + ~ sin- 




Thus t = fji 

Initially t = and r = I : 

Finally, then, 



fr-H + s s-sm- 




For purposes of computation, a better form of this equation 
is the following : 



(3) 



EXERCISES* 



1. If the earth had no atmosphere, with what velocity would 
a stone have to be projected from the earth's surface, in order 
not to come back? 

2. If the moon were stopped in its course, how long would 
it take it to fall to the earth? Regard the earth as stationary. 

Ans. 4 days, 18 hrs., 10 min. 

* In working these exercises, the following data may be used : 
Radius of the moon, ^ that of the earth. 
Mass of moon, ^ T that of earth. 
Mean distance of moon from earth, 237,000 miles. 

Acceleration of gravity on the surface of the moon, that on the surface of the 
earth. 

Diameter of sun, 860,000 miles. 

Mass of sun, 333,000 that of the earth. 

Mean distance of earth from sun, 93,000,000 miles. 

Acceleration of gravity on the surface of the sun, 905 ft. per sec. per sec. 



72 MECHANICS 

3. Solve the preceding problem accurately, assuming that the 
earth and the moon are released from rest in interstellar space 
at their present mean distance apart. Their common centre of 
gravity will then remain stationary. 

4. The same problem for the earth and the sun. 

6. If the earth and the moon were held at rest at their present 
mean distance apart, with what velocity would a projectile have 
to be shot from the surface of the moon, in order to reach the 
earth? 

6. If the earth and the moon were held at rest at their present 
mean distance apart, and a stone were placed between them at 
the point of no force and then slightly displaced toward the earth, 
with what velocity would it reach the earth ? 

7. If a hole were bored through the centre of the moon, as- 
sumed spherical, homogeneous, and at rest in interstellar space, 
and a stone dropped in, how long would it take the stone to reach 
the other side ? 

8. Show that if two spheres, each one foot in diameter and of 
density equal to the earth's mean density (specific gravity, 5.6) 
were placed with their surfaces of an inch apart and were acted 
on by no other forces than their mutual attractions, they would 
come together in about five minutes and a half. Given that the 
spheres attract as if all their mass were concentrated at their 
centres. 

9. Work Done by a Variable Force. If a force, F, constant 
in magnitude and always acting along a fixed line AB in the 
same sense, be applied to a particle,* and if the particle be dis- 
placed along the line in the direction of the force, the work done 
by the force on the particle is defined in elementary physics as 

F I W = Fl, 

A p B where I denotes the distance through which 

p eo C3 

the particle has been displaced. 

Suppose, however, that the force is variable, but varying con- 
tinuously and always acting along the same fixed line. How 
shall the work now be defined ? 

*Or, more generally, to one and the same point P of a rigid or deformable 
material body. 



MOTION OF A PARTICLE 73 

Let a coordinate be assumed on the line ; i.e. think of the line 
as the axis of x. Let the particle be displaced from A: x = a 
to B: x = 6, and let a < b. Let F, to begin with, always act 
in the direction of the positive sense along the axis. Then 

F=f(x), 

where f(x) denotes a positive continuous function of x. 

Divide the interval (a, b) up into n parts by the points x l9 
x z , , z n _i, and let X Q = a, x n = b. Then, if 

x t +i Xk = Azfc, 

the work, ATF*, done by the force in displacing the particle through 
the fc-th interval ought, in order to correspond to the general 
physical conception of work, to lie between the quantities 

FiAx and Fi'Az, 

where FJ and F' k ' denote respectively the smallest and the largest 
values of f(x) in this interval.* We have, then : 

(1) FiAx ^ ATF t ^ Fi'te. 

On writing out the double inequality (1) for k = 0, I, , 
n 1 and adding the n relations thus resulting together, we find 
that W = 2 AWk lies between the two sums : 

(2) F'^x + F(Ax + + n_, Az, 

(3) F'Jte + F('&x + + K'^Az. 
Each of these sums suggests the sum 

(4) /(* ) Az + f( Xl ) A*! + - + /(*_,) Ax n , 

whose limit is the definite integral, 

ft 

(5) lim [/(x ) A* + /(x,) Ax + + /(*._0 Ax] = f /(*) As. 

n-oo J 

a 

That W is in fact equal to this integral : 

h 

(6) W = Jf(x)dx, 

a 

follows from DuhamePs Theorem. 

* This statement is pure physics. It is the physical axiom on which the general- 
ization of the definition of work is based. More precisely, it is one of two physical 
axioms, the other being that the total work, W, for the complete interval is the sum 
of the partial works, ATT*, for the subintervals. 



74 MECHANICS 

If the force F acts in the direction opposite to that in which 
the point of application is moved, we extend the definition and 
say that negative work is done. For the case that F is constant, 
the work is now defined as follows : 

(7) W = F(b - a). 

Here, F is to be taken as a negative number equal numerically 
to the intensity of the force. 

Thus (7) is seen to hold in whichever direction the force acts, 
provided that a < 6. Will (7) still hold if 6 < a? It will. 
There are in all four possible cases : 

i) + + ii) Hi) H h 

In cases i) and ii) the force overcomes resistance, and positive 
work is done. In cases in) and iv) the force is overcome, and 
negative work is done. Hence (7) holds in all cases. 

It is now easy to see how the definition of work should be 
laid down when F varies in any continuous manner. The consider- 
ations are precisely similar to those which led to Equation (6), 
and that same equation is the final result in this, the most general, 
case : & 

W = Cf(x) dx. 

a 

Example. To find the work done in stretching a wire. Let the 
natural (or unstretched) length of the wire be I, the stretched 

length, V. Then the tension, T, is 

__, r-^-i T > i given by Hooke's Law : 

O A P B 

FIG. 59 T = \ ~~ 



where X is independent of I and V, and is known as Young's Mod- 
ulus. 

Let the wire, in its natural state, lie along the line OA, and 
let it, when stretched, lie along OB, OP being an arbitrary inter- 
mediate position. Let x be measured from A, and let x = h at 
B. Then 

T = \~ 



, TT7 /\ x , x r , 

and W = I \jdx = j I xdx = 



-==- 



MOTION OF A PARTICLE 75 

This is the work done on the wire by the force that stretches it. 
If the wire contracts, the work done by the wire on the body to 
which its end P is attached will be 



/(->!)*<" 



Xa 2 
21 



21 



EXERCISES 

1. In the problem of 7 compute the work done by the earth 
on the particle when the latter reaches the centre. 

2. A particle of mass m moves down an inclined plane. Show 
that the work done on it by the component of gravity down the 
plane is the same as the work done by gravity on the particle 
when it descends vertically a distance equal to the change in 
level which the particle undergoes. 

3. A particle is attracted toward a point by a force which 
is inversely proportional to the square of the distance from 0. 
How much work is done on the particle when it moves from a 
distance a to a distance b along a right line through 01 

4. If the earth and the moon were stopped in their courses 
and allowed to come together by their mutual attraction, how 
much work would the earth have done on the moon when they 
meet? 

5. Find the work done by the sun on a meteor when the latter 
moves along a straight line passing through the centre of the 
sun, from an initial distance R to a final distance r. 

10. Kinetic Energy and Work. Let a particle of mass m 
describe a right line with velocity v = ds/dt. Its kinetic energy 

is defined as the quantity : 

mv 2 
2 ' 

Let the particle move under the action of any force F which 
varies continuously: F = /(s). Then Newton's Second Law 
can be written in the form : 

dv f/ ^ 
fi 5 -/(). 

Hence 

mvdv = f(s)ds. 



76 MECHANICS 

Integrate this equation between the limits a and 6, denoting 
the corresponding values of v by v l and v 2 : 

6 



/ mv dv = I f(s) ds. 



The left-hand side has the value : 

mv 2 Pa 

~2~ n 

The right-hand side is, by definition, the work W done on the 
particle by the force F. Hence 



(1) 

i 
and we infer the result : 

THEOREM. The change in the kinetic energy of a particle is 
equal to the work done on it by the force which acts on it. 

This theorem expresses, in this the simplest case imaginable, 
the Principle of Work and Energy in Mechanics. By means of 
it a first integral of the equation arising from Newton's Second 
Law can be found in the case of a particle, when the force is 
known as a function of the position, and the student will do well 
to go back over the foregoing problems and exercises, and ex- 
amine their solution from this new point of view ; e.g. Equation 
(4) in 5, Equation (3) in 7, and Equation (2) in 8 are, save 
for the factor m/2, the Equation of Energy, as (1) is often called. 

EXERCISES 

Work the Exercises of 5, 7, 8, so far as possible, by the 
Method of Work and Energy. 

11. Change of Units in Physics.* To measure a quantity 
is to determine how many times a certain amount of that sub- 
stance, chosen arbitrarily as the unity is contained in a given 

* The introduction of this paragraph and the next at this stage seems to require 
justification. If these two purely physical subjects are sufficiently important to be 
taken up here, then why not, at the beginning of this chapter, the first time they 
are needed ? But if they are merely for reference, why break the unity, coherence, 
of the presentation by placing them here rather than at the end of the chapter? 
The Author feels that this is about the time when the beginner in Mechanics should 
turn his attention systematically to these subjects, for until he has some knowledge 
of the problems studied in this chapter, ho can hardly be expected to recognize the 
importance of Change of Units and of the Check of Dimensions. 



MOTION OF A PARTICLE 77 

amount of the substance.* Thus to measure the length of right 
lines is to find how many times a right line chosen arbitrarily as 
the unit of length a foot or a centimetre or a cubit is con- 
tained in a given right-line segment. The number, s, thus result- 
ing is called the length of the line. It depends on two things 
the particular line and the unit chosen. If a different unit of 
length be chosen, the same line will have a different number, 
s', assigned to it, and its length then becomes s'.f Now, for all 
lines, s' will be proportional to s : 

(1) s' oc s or s' = c s, 

where c is a constant depending on the units. It is determined 
in any given case by substituting particular values for s and s', 
known to correspond. Thus if we wish to transform from feet 
to yards, consider in particular a line which is a yard long. Here, 
s' will equal 1 and s will equal 3, so 

1 = 3c, c = i, 

and,t 

(2) ' = $8. 

Example. If a yard is the unit of length, a minute the unit 
of time, a ton the unit of mass, and a kilogramme the unit of 
force, find X in Newton's Second Law. 

We will start with Newton's Equation in the English units : 

^ 2 <? 

(3) *<y = 32/, 

* The word substance here may be too narrow in its connotations, for we want 
a word that will include every measurable quantity, from the length of a light- 
wave to the wheat crop of the world. Such a woid obviously does not exist, 
and so we agree to use substance in this sense as a terminus tcchnicus. 

t It would seem paradoxical to say that the same line has a length of 6 when 
the foot is the unit, and a length of 2 when the yard is the unit. But it must bo 
remembered that the length is a function of two variables, the unit being one of 
them. The attempt is sometimes made to meet the apparent difficulty by saying 
"3 ft. = 1 yd." But this makes confusion worse confounded; for 3 = 1 is not 
true, while on the other hand to try to introduce "concrete numbers," like 3 ft., 
10 Ibs., 5 sees., into mathematics, is not feasible. To try to change units in this 
way leads to blunders and wrong numerical results. There is only one kind of 
number in elementary mathematics. To attempt to qualify it as abstract, is to 
qualify that which is unique. The denominate attribute (3 ft., 10 Ibs., etc.) is part 
of the physical thing conceived ; it does not pertain to the mathematical counterpart, 
which is purely arithmetical. 

t Compare this equation with the attempted form of statement mentioned in 
the last footnote : " 1 yd. = 3 ft." It would seem to follow from that state- 
ment that ' yds. = 3s ft. But ' = . What a cheerful prospect for getting 
the right answer by that method 1 



78 MECHANICS 

and write the transformed equation in the form : 

Then the problem is to determine X'. Here, from (2) : 

Next, 

m f = km, 

i _ j. v 9000 lc m' m 

I - ft X ZOOO, lc - 20Q() , m - 2QO() 

Similarly, 

i' _ ? = $ 

60' J 2.20' 

Thus 

,d 2 s' _ 60 2 d 2 s 
m "^ - 2000*X3 m ^ 

XT = __L_\'/ 

*j 220 A;- 

The left-hand sides of these equations are equal by (4). On 
equating the right-hand sides and dividing by (3) we find : 

60 2 X' 



2000 X 3 2.20 X 32' 



X' = 422.4.* 



On dropping the primes, Newton's Second Law, written in the 
new units, appears in the form : 



EXERCISES 

1. If the units of length, time, and mass are respectively a mile, 
a day, and a ton, compute the absolute unit of force in pounds. 

2. If the acceleration of gravity is 981 in the c.g.s. system, 
compute g in the English system. 

3. If the acceleration of gravity is 32.2 in the English system, 
compute g in the c.g.s. system. 

* More precisely, the result should bo tabulated as : 

X' = 4.2 X 10 2 , 
since the data, namely, X - 32, are correct only to two significant figures. 



MOTION OF A PARTICLE 79 

4. If the unit of force be a pound, the unit of time a second, 
and the unit of length a foot, explain what is meant by the absolute 
unit of mass, and show that it is equal (nearly) to 32 Ibs. 

6. Formulate and solve the same problem in the decimal 
system. 

6. If the unit of mass is a pound, the unit of length, a foot, and 
the unit of force, a pound, find the absolute unit of time. 

Arts. .176 sees. 

12. The Check of Dimensions. The physical quantities that 
enter in Mechanics can be expressed in terms of the units of 
Mass [Af], Length [L], and Time [7"]. Thus velocity is of the 
dimension length/time, or L/T = LT~ l . Acceleration has the 
dimension LT~ 2 , and force, the dimension ML/T~*. 

When, an equation is written in literal form, as 



each term must have the same dimension. For, such an equation 
remains true, no matter what the units of mass, length, and time 
may be; and if two terms had different dimensions in any one 
of the fundamental quantities (mass, length, time), a change 
of units would lead to a new equation not in general equivalent 
to the old one. 

This principle affords a useful check on computation. Thus, 
if an ellipse is given by the equation : 



all the quantities x, y, a, b are of dimension one in length, or L. 
The dimension of its area must be L 2 ; and it is, for A = irab. 
The volume of the ellipsoid of revolution corresponding to rota- 
tion about the axis of x should be of dimension L 3 , and it is : 

V = 7ra6 2 . 

This principle affords a useful check on putting in or leaving 
out g, when problems are formulated literally. Thus in the 
Example of 3, if we had forgotten our g in writing down the 
right-hand side, the check of dimensions would immediately 
have shown up the oversight. For, the left-hand member is of 
dimension ML/T~~*\ hence every term on the right must have 



80 MECHANICS 

this same dimension. It does, in the correct equation of the text. 
It is, of course, only when all the quantities which enter are in 
literal form, that the check can be used. If some are replaced 
by numbers, the check does not apply. 

Observe that in computing the dimension of a derivative, like 
d 2 s/dt 2 , we may think of the latter as a quotient, the numerator 
being a difference, and hence of the dimension of the dependent 
variable, while the denominator is thought of as a power. 

EXERCISES 

Determine the dimension of each of the following quantities: 

1. Kinetic energy. Ans. ML 2 T~ 2 . 

2. Work. Ans. ML 2 T~ 2 . 

3. Moment of inertia. Ans. ML 2 . 

4. Momentum. Ans. MLT~ l . 
6. Couples. Ans. ML 2 T' 2 . 

6. Volume density. Ans. ML~ Z . 

7. Surface density. Ans. ML* 2 . 

8. Line density. Ans. ML" 1 . 

9. The acceleration of gravity. Ans. LT~ 2 . 

10. The wind resistance can often be assumed proportional 
to the square of the velocity. If it is written as cv 2 , what is 
the dimension of c? Ans. ML~ l . 

11. In Question 10, what is the answer when the wind re- 
sistance is taken per square foot of surface exposed ? 

12. Check the dimensions in each equation occurring in 3. 

13. In 4, Equation (3), the check fails. Explain why. 

14. What are the dimensions of Young's Modulus? 

15. In the Example treated in 8, we wished to find the velocity 
of the stone at the centre of the earth in miles per second. But 
if we substituted for R, in the formula (dr/df) 2 = gR, the value 
of R in miles (i.e. 4000), we obtained a wrong answer, even though 
the dimensions of both sides of this equation are the same, namely, 
L 2 /T~ 2 . Explain why, and show how Formula (2), which is 
one hundred per cent literal, can be used to yield a correct result, 
when R = 4000. 

16. Examine each equation in 8 as to whether the Check 
of Dimensions is applicable. 



MOTION OF A PARTICLE 81 

13. Motion in a Resisting Medium. When a body moves 
through the air or through the water, these media oppose re- 
sistance, the magnitude of which depends on the velocity, but 
does not follow any simple mathematical law. For low velocities 
up to 5 or 10 miles per hour, the resistance R can be expressed 
approximately by the formula : 

(1) R = av, 

where a is a constant depending both on the medium and on the 
size and shape of the body, but not on its mass. For higher 
velocities up to the velocity of sound (1082 ft. a sec.) the formula 

(2) R = cv* 

gives a sufficient approximation for many of the cases that arise 
in practice. We shall speak of other formulas in the next para- 
graph. 

Problem 1. A man is rowing in still water at the rate of 3 miles 
an hour, when he ships his oars. Determine the subsequent 
motion of the boat. 

Here Newton's Second Law gives us : 

/o\ dv 

(3) m^=-av. 

TT j* m dv 
Hence at = , 

a v 

/A\ A m i V Q 

(4) t = - log-^ 

where V Q is the initial velocity, nearj^^Bft. a sec. 
To solve (4) for v, observe that 

a * i *>o 

= log--, or 

m v v 

Hence 

_at 

(5) 9 v = V Q e . 

It might appear from (5) that the boat would never come to 
rest, but would move more and more slowly, since 

_at 

lim e~ = 0. 

= 00 

We warn the student, however, against such a conclusion. For 
the approximation we are using, R = av, holds only for a limited 



82 MECHANICS 

time, and even for that time is at best an approximation. It 
will probably not be many minutes before the boat is drifting 
sidewise, and the value of a for this aspect of the boat would 
be quite different, if indeed the approximation K = av could 
be used at all. 
To determine the distance travelled, we have from (3) : 

dv 

mv~r = av, 
ds 

and consequently : 

(6) = o-^. 

Hence, even if the above law of resistance held up to the limit, 
the boat would not travel an infinite distance, but would ap- 
proach a point distant 



feet from the starting point, the distance traversed thus being 
proportional to the initial momentum. 

Finally, to get a relation between s and t, integrate (5) : 

ds -? 



/>7\ ffiVn /1 ~m\ 

(7) 8 = -(l - e m ). 

From this result is also evident that the boat will never cover 
a distance of S ft. while the above approximation lasts. 

EXERCISE 

If the man and the boat together weigh 300 Ibs. and if a steady 
force of 3 Ibs. is just sufficient to maintain a speed of 3 miles 
an hour in still water, show that when the boat has gone 20 ft., 
the speed has fallen off by a little less than a mile an hour. 

Problem 2. A drop of rain falls from a cloud with an initial 
velocity of v ft. a sec. Determine the motion. 

We assume that the drop is already of its final size, not 
gathering further moisture as it proceeds, and take as the 
law of resistance : 

R = ct; 2 . 



MOTION OF A PARTICLE 83 

The forces which act are i) the force of gravity, mg, downward, 
and if) the resistance of the air, cv 2 , upward. As the coordinate 
of the particle we will take the distance AP, Figure 60, which 
it has fallen. Then, Newton's Second Law becomes : 

dv , A 

m-jj = mg cv 2 . 

TT dv mg cv 2 

Hence v~r = , 

as m 

cv* 

mv dv 



mg cv*' 



s = - log (mg - cv 2 ) + <7, 



and thus finally FIG. 60 

/ON W i m <7 00 

(8) s = 5- log - -t' 

v 7 2c m# cv 2 

Solving for v we have 



mg cv 2 

(9) ^gg-^-^g 

v y 



When s increases indefinitely, the last term approaches as 
its limit, arid_hence the velocity v can never exceed (or quite 
equal) v Vmg/c ft. a sec. This is known as the limiting velocity. 
It is independent of the height and also of the initial velocity, and 
is practically attained by the rain as it falls, for a rain drop is 
not moving sensibly faster when it reaches the ground than it was 
at the top of a high building. 

EXERCISES 

1. Work Problem 2, taking as the coordinate of the rain drop 
its height above the ground. 

2. Find the time in terms of the velocity and the velocity in 
terms of the time in Problem 2. 

3. Show that, if a charge of shot be fired vertically upward, 
it will return with a velocity about 3 times that of rain drops 



84 MECHANICS 

of the same size ; and that if it be fired directly downward from 
a balloon two miles high, the velocity will not be appreciably 
greater. 

4. Determine the height to which the shot will rise in Question 
3, and show that the time to the highest point is 



where v is the initial velocity. 

14. Graph of the Resistance. The resistance which the at- 
mosphere or water opposes to a body of a given size and shape 
can in many cases be determined experimentally with a reason- 
able degree of precision and thus the graph 
of the resistance : 




JL can be plotted. The mathematical problem 
^ ' 2 then presents itself of representing the curve 

with sufficient accuracy by means of a simple 
function of v. In the problem of vertical motion in the atmos- 
phere, Problem 2, 13, 

dV ^ f/ \ 

m -^ = mg f(v), 

according as the body is going up or coming down, s being meas- 
ured positively downward. Now if we approximate to f(v) by 
means of a quadratic polynomial or a fractional linear function, 



or 



we can integrate the resulting equation readily. And it is obvi- 
ous that we can so approximate, at least, for a restricted range 
of values for v. 

Another case of interest is that in which the resistance of the 
medium is the only force that acts, as in Problem 1 : 

dv ff , 
m _-/(). 

A convenient approximation for the purposes of integration is 

/() = av b . 



MOTION OF A PARTICLE 85 

Here a and b are merely arbitrary constants, enabling us to im- 
pose two arbitrary conditions on the curve, for example, to 
make it go through two given points, and are to be determined 
so as to yield a good approximation to the physical law. Some- 
times the simple values 6 = 1, 2, 3 can be used with advantage. 
But we must not confuse these approximate formulas with simi- 
larly appearing formulas that represent exact physical laws. 
Thus, in geometry, the areas of similar surfaces and the volumes 
of similar solids are proportional to the squares or cubes of cor- 
responding linear dimensions. This law expresses a fact that 
holds to the finest degree of accuracy of which physical measure- 
ments have shown themselves to be capable and with no restric- 
tion whatever on the size of the bodies. But the law R = av 2 
or R = cv* ceases to hold, i.e. to interpret nature within the limits 
of precision of physical measurements, when v transcends certain 
restricted limits, and the student must be careful to bear this 
fact in mind. 

EXERCISES 

Work out the relations between v and s, and those between 
v and I, if the only force acting is the resistance of the medium, 
which is represented by the formula : 

1. R = a + bv + cv\ 2. R = ~-~ V -- 3. R = av*. 

7 + dv 

4. Show that it would be feasible mathematically to use the 
formulas of Questions 1 and 2 in the case of the falling rain drop. 

5. A train weighing 300 tons, inclusive of the locomotive, can 
just be kept in motion on a level track by a force of 3 pounds 
to the ton. The locomotive is able to maintain a speed of 60 
miles an hour, the horse power developed being reckoned as 1300. 
Assuming that the frictional resistances arc the same at high 
speeds as at low ones and that the resistance of the air is pro- 
portional to the square of the velocity, find by how much the 
speed of the train will have dropped off in running half a mile 
if the steam is cut off with the train at full speed. 

6. A man and a parachute weigh 150 pounds. How large 
must the parachute be that the man may trust himself to it at 
any height, if 25 ft. a sec. is a safe velocity with which to reach 
the ground? Given that the resistance of the air is as the square 



86 MECHANICS 

of the velocity and is equal to 2 pounds per square foot of oppos- 
ing surface for a velocity of 30 ft. a sec. 

Ans. About 12 ft. in diameter. 

7. A toboggan slide of constant slope is a quarter of a mile 
long and has a fall of 200 ft. Assuming that the coefficient 
of friction is T Q, that the resistance of the air is proportional 
to the square of the velocity and is equal to 2 pounds per square 
foot of opposing surface for a velocity of 30 ft. a sec., and that 
a loaded toboggan weighs 300 pounds and presents a surface 
of 3 sq. ft. to the resistance of the air ; find the velocity acquired 
during the descent and the time required to reach the bottom. 

Find the limit of velocity that could be acquired by a tobog- 
gan under the given conditions if the hill were of infinite length. 
Ans. (a) 68 ft. a sec. ; (b) 30 sees. ; (c) 74 ft. a sec. 

8. The ropes of an elevator break and the elevator falls with- 
out obstruction till it enters an air chamber at the bottom of 
the shaft. The elevator weighs 2 tons and it falls from a height 
of 50 ft. The cross-section of the well is 6 X 6 ft. and its depth 
is 12 ft. If no air escaped from the well, how far would the 
elevator sink in? What would be the maximum weight of a 
man of 170 pounds? Given that the pressure and the volume 
of air when compressed without gain or loss of heat follow the 

law : pv l - 4l = const., 

and that the atmospheric pressure is 14 pounds to tho square 
inch. 

9. In the early days of modern ballistics the resistance of 
the atmosphere to a common ball was determined as follows. 
A number of parallel vertical screens were set up at equal dis- 
tances, the ball was shot through them (with a practically hori- 
zontal trajectory), and the time recorded (through the breaking 
of an electric circuit) at which it cut each screen. Explain the 
theory of the experiment, and show how points on tho graph of 
the resistance as a function of the velocity could be obtained. 

16. Motion in a Plane and in Space. Vector Velocity. When 
a point P moves in a plane or in space, its position at any instant 
can be represented by its Cartesian coordinates : 

(1) *-/(*), 2/ 



MOTION OF A PARTICLE 



87 




where the functions are continuous, together with any deriva- 
tives we shall have occasion to use. 

The velocity of P has been defined as ds/dt. For, hitherto, 
we have regarded the path as given, and it was a question merely 
of the speed and sense of description of the path. But now we 
need more. We need to put into evidence the direction and 
sense of the motion, and so we extend the idea, defining velocity 
more broadly as a vector. Lay off on the tangent to the path, 
in the sense of the motion, a directed line segment whose length 
is the speed of the point, and let the vector thus determined be 
defined as the vector velocity of the point P. 

Composition and Resolution of Velocities. A mouse runs across 
the floor of a freight car. To determine the velocity of the mouse 
in space, if the velocity of the car is u, 
and the velocity of the mouse relative 
to the car is v. 

Let the mouse start from a point P 
on one side of the car and run across 
the floor in a straight line with constant 
velocity, v, relative to the car. Let Q 
be tho point she has reached at the end 
of t seconds. Then p ~ _ 

Let the velocity, u, of the train be constant, and let be the 
initial position of P. Then 

OP = ut. 

In Figure 62, the line OA represents the vector velocity u of 
the train, and AB represents the vector velocity v of the mouse 
relative to the freight car. Their geometric, or vector, sum is 
represented by 07?. From similar triangles 
it appears that the path of the mouse in 
space is the right line through and 5, 
and that her velocity in space is the vector 
OB, or u + v. 

Thus her velocity in space may be de- 
scribed, from analogy with the parallelo- 
gram of forces, as the resultant of the two component velocities, 
u along the direction of OA and v along the direction OC through 
O parallel to A. 



ut 



FIG. 62 




FIG. 63 



88 MECHANICS 

Similarly, any vector velocity may be resolved into two com- 
ponent velocities along any two directions complanar with the 
given velocity ; Fig. 63. 

The extension to space is obvious. Any three non-complanar 
vector velocities can be composed into a single velocity by the 
parallelepiped law. And conversely any given vector velocity 
can be decomposed into three component vector velocities along 
any three non-complanar directions. 

The General Case. Returning now to the general case of motion 
in a plane or in space, we may define the average vector velocity for 
the At seconds succeeding a given instant as the vector * (PP') 
divided by A, or the vector (PQ) : 



When At approaches as its limit, the length of this vector, 
namely, the chord PP , divided by At, approaches the speed of 
the point at P ; or, 

r ~P**' r As n n 

hm - = hm = Dts = v, numerically. 

A = O At AJ-=O At 

Moreover the direction of the variable vector (PQ) approaches 
a fixed direction as its limit. And so the variable vector (PQ) 
approaches a fixed vector, v, as its limit, or 



lim --V- = lim (PQ) = v. 

A* = At AZ = 

This vector, v, is defined as the vector velocity of the point P. 

Cartesian Coordinates. To prove that the above limit actually 
exists, consider the components of (PP') and (PQ) along the. 
axes. These arc : 

i A# Ay Az 
Ax, Ay, A* and -, -, - 

The last three variables approach limits : 

lim -7 = Dix, lim --7 = D t y, lim ~ = Dtz. 

A-0 At Af-0 At A/=*0 At 

Hence (PQ) approaches a limit, v, and the components of v along 
the axes are : 

* When it is not feasible to represent vectors by bold face type, the ( ) 
notation may be used, as: (PP') or, later, (a). The student should draw the 
figure which represents the vectors (PP') and (PQ)> 



MOTION OF A PARTICLE 89 

dx __ dy __ dz 

Vx ~Tt' Vv ~ ~dt' Vz " ' 

These equations admit the following physical interpretation. 
Consider the projections, L, Af, TV, of the point P on the axes of 
coordinates. The velocities with which these points are moving 
along the axes are precisely dx/dt, dy/dt, and dz/dt. And so we 
can say : The projections of the vector velocity v along the axes are 
equal respectively to the velocities of the projections. 

Finally, observe that, just as the average vector velocity ap- 
proaches the actual vector velocity as its limit, so the projections 
of the average vector velocity approach the projections of the 
actual vector velocity as their limits. 

Remark. The student may raise the question : If v x , v y , and 
v z are the components of the vector velocity, v, are they not, 
therefore, themselves vectors, and should they not be written 
as such, v z , v y , v z ? Yes, this is correct. But it does not con- 
flict with the other view of v x , v y , and v z as directed line segments 
on the axes of x, y, and z. For, a system of vectors whose direc- 
tion (but not sense) is fixed, constitute a system of one-dimen- 
sional vectors, and these are equivalent to directed line segments, 
since the two systems stand in a one-to-one relation to each 
other. One-dimensional vectors can be represented arithmeti- 
cally by the ordinary real numbers, positive, negative, and zero. 

EXERCISES 

1. Show that, if polar coordinates in the plane are used, the 
component velocities along and orthogonal to the radius vector 

are respectively : 

dr dB 



2. A point moves on the surface of a sphere. Show that 

dB . A d<p 



where 6 and <p denote respectively the co-latitude and the longi- 
tude. 

3. A point moves in space. Show that 
dr dB 



where r, 6, <p are the spherical coordinates of the point. 



90 MECHANICS 

16. Vector Acceleration. Let a point describe a path, as 
in 15. By the vector change in its velocity is meant the vector 

(1) Av = v' - v, 

cf. Fig. 65, p. 96. The average vector acceleration is defined as the 

vector 

Av 

AT 

When A approaches 0, the average vector acceleration approaches 
a limiting value, and this limiting vector is defined as the vector 
acceleration of the point : 

/ \ r Av 
(a) = hm 
Ar=o At 

Cartesian Coordinates. The components of the vector acceler- 
ation along the Cartesian axes, at x , a^, and a z , arc readily com- 
puted. For, the components of the vector (1) along the axes 
are respectively : 

v' x v x v'y v y v' z v z 



AJ ' AJ ' AZ 

As in the case of velocities, the components of the limiting vector 
and the limits approached by the components of the variable 
vector are respectively equal.* Hence 

,. At> z ~ ,. Av y ~ .. Av z ~ 

a x = hm = Dtv x , a v = hm = Dtv v , a z = hm - = Dtv t , 

A/ = *** A/ = &t A/ = At 

or: 

d' 2 z 



Osculating Plane and Principal Normal.] Let a vector r be 
drawn from an arbitrary fixed point of space to the variable 
point P that is tracing out the curve (1), 15. Then 

dr . 

v --a = *- 

Let s be the arc, measured in the sense of the motion ; and let 



. 
ds 

* This theorem is true of any vector which approaches a limit, as the student 
can readily verify. 

f Cf. the Author's Advanced Calculus, p. 304, 8. 



MOTION OF A PARTICLE 91 

Then r' is a unit vector lying along the tangent and directed 
in the sense of the motion. Furthermore, 



= r 
ds 



is a vector drawn along the principal normal, toward the con- 
cave side of the projection of the curve on the osculating plane, 
and its length is the curvature, K, at P. 
On the other hand, the acceleration 



dv , dsdr 

= and *-__ 



Hence 



EXERCISES 

1. A point describes a circle with constant velocity. Show 
that the vector acceleration is normal to the path and directed 
toward the centre of the circle, and that its magnitude is 

" 2 2 

, or or r. 

2. Show that, when a point is describing an arbitrary plane 
path, the components of the vector acceleration along the tangent 
and normal are : <j 2 s v* 

at = w' an = ? 

whoro p denotes the radius of curvature, and the component <x n 
is directed toward the concave side of the curve. 

3. A point describes a cycloid, the rolling circle moving forward 
with constant velocity. Show that the acceleration is constant 
in magnitude and always directed toward the centre of the circle. 

4. Prove by vector methods that, in the case of motion in 



where a r , a denote the components of the acceleration along 
and perpendicular to the radius vector. 

Use the system of -ordinary complex numbers, a + bi, where 

i = V 1, and set . 

' r = re 6 \ 

5. Obtain the same results by geometric methods. 



92 MECHANICS 

17. Newton's Second Law. Let a particle move under the 
action of any forces, and let F be their resultant. Let (a) be 
its vector acceleration. Then Newton's Second Law of Motion 
asserts that the mass times the vector acceleration is proportional to 
the vector force , or, if the absolute unit of force is adopted, 
(1) m(a) = F. 

In Cartesian coordinates the law becomes : 

W>-J7Z = X, 



(2) 

t d?z 

If, in particular, X, Y, Z are continuous functions of x, y, z, 
dx/dt, dy/dt, dz/dt, and t y it then follows from the theory 
of differential equations that the path is uniquely determined 
by the initial conditions; i.e. if the particle is projected from a 
point (z , 2/o> ZG) with a velocity whose components along the axes 
are (u^ v , w ), the path is completely determined. This remark 
is striking when one considers that the corresponding theorem 
is not true if one determines the motion by means of the principle 
of Work and Energy; cf. the Author's Advanced Calculus, p. 351, 
Singular Solutions. The essential point here is that Equa- 
tions (2) never admit a singular solution, whereas the equations 
of Work and Energy do. 

In the more general cases it is also seen that the path is uniquely 
determined by the initial conditions. This statement is con- 
firmed in the case of each of the examples considered below. 
For a general treatment, cf. Appendix A. 

Osculating Plane. The force, F, always lies in the osculating 
plane of the path. For, from 16, and Equation (1) above, 

Hence we can resolve F into a component T along the path and a 
component N along the principal normal, and we shall then have : 

y"72 o tYllfi 

m = T = N 

where p = l//c. 



MOTION OF A PARTICLE 



93 



EXERCISE 

Show that (r' x r") F = 0. 

Hence, in Cartesian coordinates, 

-(z'x")Y+(x'y")Z = 0, 



where 
and 



y'z"-z'y", 



etc. 



/ dx fr 

ff 1 f 

JU ~; . JU 

ds 



etc. 



18. Motion of a Projectile. Problem. To find the path of a 
projectile acted on only by the force of gravity. 

The degree of accuracy of the approximation to the true motion 
obtained in the following solution depends on the projectile and 
on the velocity with which it moves. For a cannon ball it is 
crude, though suggestive, whereas for the 16 Ib. shot, used in 
putting the shot, it is decidedly good. 

Hitherto we have known the path of the body; here we do 
not. The path will obviously be a plane curve, and so Newton's 
Second Law of Motion becomes : 



m 



dt 2 



where X , Y are the components of the resultant force along the 
axes, measured in absolute units. 
In the present case X = 0, Y = mg, and we have 



(2) 






FIG. 64 



If we suppose the body projected from with velocity V Q at 
an angle a with the horizontal, the integration of these equations 

ives: dx 
dt 



-jj = (J = VQ cos a, x = v 1 cos a ; 



^ = v Q sin a - 0tf , y = V / sin a - 



94 MECHANICS 

Eliminating t we get : 

OX" 

(3) y = x tan a - -^- 5- 

2^ cos 2 a 

The curve has a maximum at the point A : (z,, t/J, 
t$ sin a cos a #?, sin 2 a 

/M _ U /% U 

*> ff ' *> - ~2T~ 

Transforming to a set of parallel axes through A, we have : 
x = x 1 + a?!, y = y' + y lt 



V ' * 2 2 COS 2 n, 

&UQ LUo Cc 

This curve is a parabola with its vertex at A. The height 
of its directrix above A is v\ cos 2 a/2</, and hence the height 
above of the directrix of the parabola represented by (3) is 

vl sin 2 a . v% cos 2 a _ v% 

~~2g~ + 2i~ " 27' 

The result is independent of the angle of elevation a, and so 
it appears that all the parabolas traced out by projectiles leaving 
with the same velocity have their directrices at the same level, 
the distance of this level above being the height to which the 
projectile would rise if shot perpendicularly upward. 

EXERCISES 

1. Show that the range on the horizontal is 

R = sin 2a, 
j/ 

and that the maximum range R is attained when a = 45 : 

~ g' 
The height of the directrix above is half this latter range. 

2. A projectile is launched with a velocity of V Q ft. a sec. and 
is to hit a mark at the same level and within range. Show that 
there are two possible angles of elevation and that one is as much 
greater than 45 as the other is less. 

3. Find the range on a plane inclined at an angle j3 to the 
horizon and show that the maximum range is 

* ~ ~g 1 + sin 



MOTION OF A PARTICLE 95 

4. A small boy can throw a stone 100 ft. on the level. He 
is on top of a house 40 ft. high. Show that he can throw the 
stone 134 ft. from the house. Neglect the height of his hand 
above the levels in question. 

6. The best collegiate record for putting the shot was, at 
one time, 46 ft. and the amateur and world's record was 49 ft. 
Gin. 

If a man puts the shot 46 ft. and the shot leaves his hand at 
a height of 6 ft. 3 in. above the ground, find the velocity with 
which he launches it, assuming that the angle of elevation a is 
the most advantageous one. Am. v = 35.87. 

6. How much better record can the man of the preceding 
question make than a shorter man of equal strength and skill, 
the shot leaving the latter's hand at a height of 5 ft. 3 in. ? 

7. Show that it is possible to hit a mark B : (x6, 2/&), provided 



8. A revolver can give a bullet a muzzle velocity of 200 ft. 
a sec. Is it possible to hit the vane on a church spire a quarter 
of a mile away, the height of the spire being 100 ft. ? 

9. It has been assumed that the path of the projectile is a 
piano curve. Prove this assumption to be correct by using all 
three Equations (2), 17. 

19. Constrained Motion. Let a particle be constrained to 
move in a given curve, like a smooth bead that slides on a wire. 
Consider first the case of a plane curve. Let the component 
of the resultant of all the forces along the tangent be T and along 
the normal be N. Then Newton's Second Law of Motion, 17, 
gives the following equations : 



(1) 

mv 



2 = N. 
P 



The proof given in 17 was based on vector analysis. We will 

give one for the plane case without the use of vector methods. 

Geometric Proof. Compute the components of the vector 

acceleration along the tangent and along the normal. Let <p 



96 



MECHANICS 



be the angle which the tangent has turned through in passing 
from P to P' . Then the component of Av along the tangent 

will be 

v f cos tp v = (t; + Av) cos <p v 

= Av cos <p v (1 cos <p). 
By the definition of curvature, 




K = lim~r, p = lim 
PP' 



PP' 



Now, the component of the average ac- 
celeration along the tangent is 

v f cos & v Av 1 cos (p 

TT = -r- COS <f> V - 

At At At 

Let At approach 0. Then <p approaches 0, and the limit of the 
first term on the right is 

/,. AZA/V \ ~ 

f lim Mlimcos^J = D t v. 

To evaluate the limit of the second term, write 

1 cos y? __ 1 cos <p jp_ As 
At <p As At 

The first factor approaches 0, and the second and third factors 
remain finite, since each approaches a limit. Hence the limit 
of the right hand side is 0. 
We have proved, then, that 

,. v f cos <p v ~ 
lim = Dtv, 

and thus the first of Equations (1) is established. 

To obtain the second of Equations (1), consider the component 
of the average acceleration along the normal, or 



This can be written as 



v sm <p 
At 

; sin <p (?_ As 
v 



_ 
<p As At' 



MOTION OF A PARTICLE 97 

where s is assumed to increase with t. The limit of this product 
is seen to be : i 2 

v X 1 X - X v = -, 
P P 

and this proves the theorem. 

The component N measures the reaction of the curve. It is 
the centripetal force due to the motion. 

The foregoing analysis yields the first of Equations (1) for 
twisted curves. 

EXERCISE 

Use the present geometric method to obtain the formulas : 

1 d 



where a r , ot e denote respectively the components of the vector 
acceleration along and perpendicular to the radius vector. 

20. Simple Pendulum Motion. Consider the simple pendu- 
lum. Here ^ s 

m -772 = - mg sin 0, 
at 

and since s = 1 0, 

This differential equation is characteristic for Simple Pendulum 
Motion. We can obtain a first integral by the method of 7 : 



2g . de 

~~T: 77^ ~T~ sin u -jr. 
dt dt 2 I at 



= cos + C, 
where a is the initial angle ; hence 
(2) ^ = ^(cos0-cos). 

The velocity in the path at the lowest point 
is I times the angular velocity for = 0, or 
V20Z (1 cos a), and is the same that would have been acquired 
if the bob had fallen freely under the force of gravity through the 




MECHANICS 



same difference in level. Equation (2) is virtually the Integral 
of Energy. 

If we attempt to obtain the time by integrating Equation (2), 
we are led to the equation : 

de 




20 J Vcos cos a 



This integral cannot be expressed in terms of the functions at 
present at our disposal. It is an Elliptic Integral.* When 0, 
however, is small, sin 6 differs from 6 by only a small percentage 
of either quantity, and hence we may expect to obtain a good 
approximation to the actual motion if we replace sin 6 in (1) by : 



(3) 



_ g 
-~ 



This latter equation is of the type of the differential equation 
of Simple Harmonic Motion, 7, A), n 2 - having here the value 
g/l. Hence, when a simple pendulum swings through a small 
amplitude, its motion is approximately harmonic and its period 
is approximately 



9 

The Tautochrone. A question that interested the mathema- 
ticians of the eighteenth century was this : In what curve should 
a pendulum swing in order that the period of oscillation may bo 
absolutely independent of the amplitude? It turns out that 
the cycloid has this property. For, the differential equation of 

motion is 

d z s 




FIG. 67 



where $ is measured from the lowest 
' point, and since 

s = 4a sin r, 

, d*s g 

we have -j-z = -~ s. 
at 2 4a 



* Cf. the author's Advanced Calculus, Chapter IX, page 195, where this integral 
is reduced to the normal form. 



MOTION OF A PARTICLE 



99 



This is the differential equation of Simple Harmonic Motion, 
7, A), and hence the period of the oscillation, 



9 

is independent of the amplitude. 

A cycloidal pendulum may be constructed by causing the cord 
of the pendulum to wind on the evolute of the path. The resist- 
ances due to the stiffness of the cord as it winds up and unwinds 
would thus be slight ; but in time they would become appreciable. 

21. Motion on a Smooth Curve. Let a bead slide on a 
smooth wire under the force of gravity. Consider first the plane 
case. Choosing the axes as indicated, we have : 



(1) 
Hence 



dt* 



dx 
ds 



_ 9 

2 ~ g 



~ds~dt 



Integrating this equation with respect 
to /, we find : 



If we suppose the bead to start from 
rest at A, then 

= 2gx Q + C, 



\A:(x Q ,y ) 




FIG. 68 



(2) 







But the velocity that a body falling freely from rest a distance of 
x x attains is expressed by precisely the same formula. 

In the more general case that the bead passes the point A 
with a velocity v we have : 



(3) 



eg = 2gx<> + C, 
t> 2 - eg = 2g (x - z ). 



Thus it is seen that the velocity at P is the same that the bead 
would have acquired at the second level if it had been projected 
vertically from the first with velocity . 



100 MECHANICS 

The theorem also asserts that the change in kinetic energy is 
equal to the work done on the bead ; cf. 10. 

If the bead starts from rest at A, it will continue to slide till 
it reaches the end of the wire or comes to a point A' at the same 
v* >^L level as A In the latter case it will in gen- 
eral just rise to the point A 1 and then retrace 
its path back to A. But if the tangent to the 
FIG. 69 curve at A ' is horizontal, the bead may 

approach A 1 as a limiting position without ever reaching it. 

EXERCISES 

1. A bead slides on a smooth vertical circle. It is projected 
from the lowest point with a velocity equal to that which it would 
acquire in falling from rest from the highest point. Show that 
it will approach the highest point as a limit which it will never 
reach. 

2. From the general theorem (2) deduce the first integral 
(2) of the differential equation (1), 20. 

Space Curves. The same treatment applies to space of three 
dimensions. It is interesting, however, to give a solution based 
on Cartesian coordinates. Choose the axis of x as before positive 
downward. Then we have : 



(4) 



. D 
~dT* = "% + R *> 

d*y _ D 
~* ~ "' 



where R x , R v , R t are the components of the reaction R of the wire 
along the axes. Since R is normal to the curve, we have : 

< s -S+*-8 + *!- 

To integrate Equations (4) multiply through respectively by 
dx/dty dy/dt, dz/dt and add. We thus find, with the aid 
of (5): 



MOTION OF A PARTICLE 101 

But 

2 /efo\ 2 . (dy\ 2 /dz\* 

" 2 = (&) + U) + b) 

Hence (6) reduces to 

(7) ^ m d (v 2 ) = mg dx. 
On integrating this equation, we find : 

/o\ mvZ mv a / \ 

(8) -7j --- 2^ = "V (* - *<>) 

This is precisely the Equation of Energy. It could have been 
written down at the start from the Principle of Work and Energy. 
It is the generalization of (2) for space curves. 

EXERCISE 

A bead slides on a smooth wire in the form of a helix, axis 
vertical. Determine the reaction of the wire in magnitude and 
direction. 

22. Centrifugal Force. When a particle of mass m describes 
a circle with constant velocity, the acceleration is directed toward 
the centre, and its magnitude is 




The force which holds the particle in its path is, 
therefore, normal to the path and directed inward. 
Its magnitude is 

, r mv 2 9 FIG. 70 

N = - = mco 2 r. 
r 

Why, then, the term " centri/u^aif force" the force that "flees 
the centre"? The explanation is a confusion of ideas. If the 
mass is held in its path by a string fastened to a peg at the centre, 
0, does not the string tug at in the direction OP away from the 
centre and is not this force exerted by the particle in its attempt, 
or tendency, to fly away from the centre? The answer to the 
first question is, of course, "Yes." Now one of the standard 
methods of the sophists is to begin with a question on a non- 
controversial point, conceded without opposition in their favor, 
and then to confuse the issue in their second question "and 
is not this force exerted by the particle?" 



102 MECHANICS 

Matter cannot exert force, for a force is a push or a pull, and 
matter can neither push nor pull ; it is inert. The particle does 
not pull on the string, the string pulls on the particle. But even 
this statement will be accepted only half-heartedly, if at all, 
by people who have not yet grasped the basic idea of the science 
of Mechanics the study of the motion of matter under the 
action of forces. What comes first is a material system solid 
bodies, particles, laminae and material surfaces, wires, any combi- 
nation of these things, including even deformable media (hydro- 
dynamics, elasticity) and then this system is acted on by 
forces. 



ISOLATE THE SYSTEM 



The man who first uttered these words deserves a monumentum 
aere. In the present case there are two systems, each of which 
can be isolated : (1) the particle ; (2) whatever the peg is attached 
to think of a smooth table, the particle going round and round 
in a horizontal circle and being held in its path by a string whose 
other end is attached to a peg at a point of the table. In the 
case of the first system, the force that acts is the pull of the string 
toward the centre, and this force is what is now-a-days described 
as "centripetal" force the force that " seeks the centre." 
The second system has nothing to do with the particle. In 
particular, this system may be the table. In that case, the floor, 
as well as gravity, exerts certain forces, and under the action of 
all the forces, the table stays at rest. The force of the string, 
varying in direction, causes the forces of the floor to vary. 

And now, after all is said and done, comes the rejoinder: "But 
the particle did pull on the string, for otherwise the string would 
not have pulled on the peg." There is no answer to these people. 
Some of them are good citizens. They vote the ticket of the 
party that is responsible for the prosperity of the country ; they 
belong to the only true church ; they subscribe to the Red Cross 
drive but they have no place in the Temple of Science ; they 
profane it. 

Example 1. A bullet weighing 1 oz. is shot into a sling, con- 
sisting of a string 5 ft. long with one end fastened at 0, the other 
end carrying a leather cup. If the velocity of the bullet is 600 ft. 
a sec., how strong must the string be, not to break? 



MOTION OF A PARTICLE 103 

The tension in the string will be o 5 ^ 

mv 2 I 



FIG. 71 



where m = ^, v = 600, r = 5 ; or 

600 2 



16X5 



4500 ; 




4500 what? pounds? No, for the force is measured in absolute 
units, or poundals, and so, to get the answer in pounds, we must 
divide by 32. The tension, then, that the string must be able 
to withstand is 141 Ibs. 

Example 2. A railroad train rounds a curve of 1000 ft. radius 
at 30 m. an hour. How high should the outer rail be raised, 
fc if the flanges of the wheels are not to 

press against either track? Standard 
gauge, 4 ft. 8| in. 

If a plumb bob is hung up in a car, 
and does not oscillate, then it should be 
at right angles to the axles of the wheels. 
It will describe its circular path in space 
under the action of two forces, namely, 
gravity, mg, downward, and the tension, 
\ T, of the string. Let the string make 

mg 7 an angle a. with the vertical. Then the 

vertical component of T just balances 
gravity, for there is no vertical motion of the bob. Hence 

T cos a. ~ mg. 

The horizontal component of T yields the normal force N which 
keeps the bob in its circular path, or 



Hence 

v 2 44 2 




Since the distance between the rails is 4 ft. 8 in., it follows that 
the outer rail must be raised 3.42 in. 



104 MECHANICS 

EXERCISES 

1. A particle weighing 4 oz. is attached to a string which 
passes through a small hole, 0, in a smooth table and carries 
a weight W at its other end. If the first weight is projected 
along the table from a point P at a distance of 2 ft. from with 
a velocity of 50 ft. a second in a direction at right angles to OP, 
the string being taut and the part below the table vertical, how 
great must W be, that the 4 oz. weight may describe a circular 
path? Ans. 9 Ibs. 12 oz. 

2. A boy on a bicycle rounds a corner on a curve of 60 ft. 
radius at the rate of 10 m. an hour, and his bicycle slips out from 
under him. What is the greatest value p, could have had ? 

Ans. Not quite |. 

3. A conical pendulum is like a simple pendulum, only it is 
projected so that it moves in a horizontal circle instead of in a 
vertical one. Show that 

Zo> 2 = g sec a. 

4. If the earth were gradually to stop rotating, how much 
would Bunker Hill Monument be out of plumb? Given, that 
the height of the monument is 225 ft. and the latitude of Charles- 
town is 42 22'. Ans. About 4 in. 

5. An ocean liner of 80,000 tons is steaming east on the equator 
at the rate of 30 knots an hour. If she puts about and steams 
west at the same rate, what is the increase in her apparent weight ? 

6. If the earth were held in her course by steel wires attached 
to the surface on the side toward the sun and evenly distributed 
as regards a cross-section by a plane at right angles to them, 
show that they would have to be as close together as blades of 
grass. It is assumed that their other ends are guided near the 
earth's surface. 

7. Show that a steel wire one end of which is made fast to 
the sun and which rotates in a plane with constant velocity, 
making one rotation in a year, could just about reach to the 
earth without breaking. Neglect the heat of the sun and all 
forces of gravitation. 

8. A steel wire 1 sq. mm. in cross-section, breaking strength 
70 kgs., is strung round the earth along the equator. Show that, 
if the earth gradually stopped rotating, the wire would snap. 



MOTION OF A PARTICLE 



105 



9. What is the smallest latitude such that the wire described 
in the preceding question, if strung round the earth on that par- 
allel, would not break ? 

10. If the earth had a satellite close by, how often would 
the latter rise and set in a day? Ans. About 18 times. 

11. A boy swings a bucket of water around in a vertical circle 
without spilling any. Does not the bucket exert a pull on the 
boy's hand ? 

Explain the situation by isolating a suitable system, namely: 
i) the bucket of water ; ii) the boy. 

23. The Centrifugal Oil Cup. A device once used for deter- 
mining the speed of a locomotive consisted of a cylindrical cup 
containing oil and caused to rotate about its axis, which was 
vertical, with an angular velocity proportional to the speed of 
the train. Let us sec how it worked. 

Suppose the oil to be rotating like a rigid body, with no cross 
currents or other internal disturbances. What will be the form 
of the free surface ? Imagine a small par- 
ticle floating on the oil. It will be acted 
on by the force of gravity, mg, downward 
and the buoyancy, B, of the oil normal to 
the surface. The resultant of these two 
forces must just yield the centripetal 
force N required to keep the particle in 
its path. Now 




N = mco 2 x. 



FIG. 73 



On the other hand, the slope of the curve is determined by the 
fact that the tangent is normal to B. Thus 

B cos T = mg, B sin r = N. 



Hence 



U'X 



or 

dx " g X ' 
It follows, then, that 

0) v-$*. 

Thus it appears that the free surface is a paraboloid of revolution 



106 MECHANICS 

To Graduate the Cup. It is easily shown that the volume of 
a segment of a paraboloid of revolution is always half the volume 
of the circumscribing cylinder. If, then, we mark the level of 
the oil when it is at rest, the height, h, to which it rises above this 
level when it is in motion will just equal the depth, h, of the 
lowest point of the surface below this point. From (1) it follows, 
then, that if a denotes the radius of the cup, 



or 



EXERCISES 

1. A tomato can 4 in. in diameter is filled with water and 
sealed up. It is placed on a revolving table and caused to rotate 
about its axis, which is vertical, at the rate of 30 rotations a sec. 
Find the pressure on the top of the can. 

Ans. The weight of a column of water 4 ft. high (nearly) 
and standing on top of the can. 

2. How great is the tendency of the can to rip along the seam? 

24. The Centrifugal Field of Force. It is possible to view the 
mechanical situation in the oil cup from a statical standpoint. 
Imagine very tiny insects crawling slowly round on tho surface 
of the oil. To them the oil and all they could sec of the walls 
and top of the cup would appear stationary, and they would 
refer their motion to the rotating space as if it were at rest. 

We can reproduce the situation, so far as statical problems 
are concerned, in a space that is actually at rest by creating a 
field of force, in which the force which acts on a particle of mass m 
distant r from a fixed vertical axis is the resultant of the force 
of gravity, mg, vertical and downward, and a force mcoV directed 
away from the axis, where co is a constant. Thus the magnitude of 
the force would be 



+ (mco 2 r) 2 = 

and it would make an angle <p with the downward vertical, where 

wV 

tan <p = 





MOTION OF A PARTICLE 107 

To bring the mechanical situation nearer to our human intui- 
tion, we might think of a large round cup, 500 ft. across at the 
top, constructed with the flooring in the form of the paraboloid 
in question and rotating with the suitable angular velocity. 
There would be a small opening at the vertex, through which 
observers could enter and leave. The view of all surrounding 
objects would be cut off, and the mechanical construction would 
be so nearly perfect that, when we were inside the cup, we should 
not perceive its motion. Suppose, for example, that the slope 
of the floor along the rim were 45. Then, since 

uPx 
tan T = , 

g 
it follows that 



~ 32 ' 

co = T 4 T (nearly), or .36. 
The time, T, of a complete revolution is given by the equation : 

27T 
- jT, 

or 

T = = 17 sees. 

0> 

Thus the cup would make nearly four revolutions a minute. 
Since co 2 /gr = ^^, the intensity of the field would be 



(0.004r) 2 , 

and upon the rim of the cup, this would amount to mgV2, or 
41 per cent greater than gravity on the fixed surface of the earth 
roughly, two-fifths more. A movie actress who was main- 
taining her weight in Hollywood, would tip the scales at, 
well, how much ? 

What we have said applies, however, only to bodies that are 
at rest in the field. When a body moves, still other forces enter, 
and these will be considered in the chapter on Relative Motion. 
Nevertheless, we can describe the motion of a projectile directly, 
since it would be a parabola in the fixed space we started with. 
Imagine a tennis court laid out with its centre at the lowest 
point of the bowl. Lob the ball from the back line to the back 
line, and watch the slice ! 



108 MECHANICS 

One may reasonably inquire concerning the engineering prob- 
lems of the construction. There will be a tendency of the cup 
to burst to fly apart, due to the "centrifugal force." Can it 
be held together by reinforcing it with steel bands round the 
outer rim, or will these have all they can do to hold themselves 
together? It turns out that only one-seventieth of the break- 
ing strength will be needed to hold the band together, thus leav- 
ing sixty-nine seventieth^ for reinforcing. 

But since at the rim the "centrifugal force" is as great as the 
force of gravity, any unbalanced load will cause the cup to tug 
on its anchorage unmercifully. A hundred men weigh approxi- 
mately 8 tons, and if they were bunched at a point of the rim, 
the reaction on the anchorage would be 8 tons. The student 
will find it interesting to compute the reaction in case a racing 
car were driven along the rim at 100 miles an hour. 

25. Central Force. Let a particle be acted on by a force 
directed toward a fixed point, O, and depending only on the 
distance from O, not on the direction. Newton's Second Law 
of Motion, 17, then becomes : 



(1 > 

d.(r*\ = 

rdt\ dt) ' 

where R is a continuous function of r. 
Law of Areas. The second equation admits a first integral : 

(2) r ^ ==h ' 

This equation admits a striking interpretation. Consider the 

area, A, swept out by the radius 
vector drawn from to the par- 
ticle. Then 

A = / r*dd, 




FIG. 74 dt ~~ dt 



MOTION OF A PARTICLE 109 

and hence 

(3) A=ft(-g, 

or, equal areas are swept out in equal times. 

We have tacitly assumed that h 5* 0. If h = 0, then (2) 
reduces to dd = 0, and the path is a straight line through 0. 

Work and Energy. The kinetic energy of the particle is 

nw^_m(W W 
W 2 " 2 W + r < 

By virtue of (2) this becomes : 



= i 

2 ~ 2 2 2 



On the other hand, the work, cf. Chap. VII, 3. 

r 

(6) TF = Cfidr. 



Hence 

I _ 

~ J? 



1 _ 2 / 

7> ~ mh*J 



This is a differential equation of the first order connecting 
r and 6, and its integral gives the form of the path. 

The Law of Nature. Newton discovered the Law of Universal 
Gravitation, which says that any two particles in the universe 
attract each other with a force proportional to their masses and 
inversely proportional to the square of the distance between 
them. This law is often referred to as the Law of Nature. 

In the present case, then, the particle is attracted toward 
with a force proportional to 1/r 2 , and so 

(8) ll^, =- 
Thus 

(9) ^ 

The Law of Energy, as expressed in the form of Equation (7), 
here becomes : 



110 MECHANICS 

where X = m/x, and C is a constant depending on the initial condi- 
tions. 

The form of this equation suggests a simplification consisting 
in substituting for r its reciprocal : 

(11) u = J- 

Thus (10) becomes : 



/io\ i 9 2/4 . ~ 

(12) ^ 5 + = - S ; + C'. 

This equation admits further reduction. Write : 



Since the left-hand side can never be negative, the right-hand 
side can be written as 5 2 , and B itself may be chosen as either 
one of the square roots. Finally, set 

* - u ~ ? 

Then (13) goes over into : 

dr 2 

(14) * + ^ - B". 

The general integral of this differential equation can be written 
in the form : 

(15) x = B cos (0 - 7), 

where y is the constant of integration. When 5 = 0, the truth 
of this statement is obvious, for then (14) reduces to 

+ * - 

de* + x u ' 
and the only solution of this differential equation is * 

x = 0. 
If S 2 * 0, then (14) yields : 

d8 = 




* We have here an example of a differential equation of the first order, handed 
to us by physics, whose general integral does not depend on an arbitrary constant, 
but consists of a unique function of alone. 



MOTION OF A PARTICLE 111 

where, however, the two signs are not necessarily the same. 
But in all cases this last equation leads to (15).* 

We set out to integrate Equation (12), and we have arrived 
at the result : 
(16) u = ~ + B cos (e - 7). 

This equation can be thrown into familiar form by taking B 
as the negative radical and setting 



where e now is the constant of integration. Thus (16) yields : 

(\7\ r = - 

1 } M 1 - ecos(0 - 7) 

The Orbit. The path of the particle is given by Equation (17). 
This is the equation of a conic referred to a focus as pole and 
having the eccentricity e. 

The Case e < 1. If e < 1, the conic is an ellipse, and the 
length of the transverse axis is 



M (1 - e*) 
Denoting the length of the semi-axes by a and 6, we have : 

h* . A 2 



- Md-e 2 )' M Vf=T' 

The distance between the foci is 

(19) c = 

The area of the ellipse is 

(20) TTOfc = 

Th 
tion: 

A = pr. 

Hence 

(21) T 2 = 47r 2 -- 

* It is worth the student's while to follow through these multiple-valued func- 
tions, that he may secure a firmer hold on the Calculus, even though the final 
result Equation (15) is simple. 



(1 - e 2 ) 1 
The periodic time T is connected with the area A by the rela- 



112 MECHANICS 

Determination of the Constants of Integration. Let the body be 
projected from the point (r, 0) = (a, 0) with an initial velocity 
VQ in a direction making an angle ft with the prime direction 
= o. To determine the orbit. 

We will mention first a general formula. Let \l/ be the angle 
from the radius vector produced to the tangent. Then 



since each side represents the component v e of the vector velocity, 
v, perpendicular to the radius vector. By virtue of (2) this 
becomes : 
(22) h = vr sin ^, 

and this is the formula we had in mind. 

To determine the constants in (17), then, write the equation 
in the form : 

/f>O\ _ r* / '-j //j \\ 

Hence 

(24) - = -^ (1 e cos 7), e cos 7 = 1 

ah* an 

Furthermore, 

du fie . 

= - sin (Q -y). 

dO h' 2 

Since 

du __ 1 dr __ i dr __ v cos \f/ 
d6 r 2 dO h dt h ' 

we have initially : 

/rt/\ M^ ^n COS p . Vi\ il COS p 

(26) T^ sin 7 = , -. e sin 7 = 

h i h M 

From (22), 

(27) h = V Q a sin j8, cos 2 ft = 1 ^- 

U i / i - 2 y^ 



Squaring the second equation in (24) and (26), and adding, 
we find by the aid of (27) : 

(28) e 



MOTION OF A PARTICLE 113 

The evaluation is now complete. By means of (27), h is deter- 
mined ; (28) then gives e, and (24) and (26) yield 7. 
From (28) we infer that 



and this equation contains the interesting result that the orbit 
will be the following conic : 

i) ellipse, if v% < ; 

ii) parabola, if v\ = ; 

Hi) hyperbola, if v% > , 

irrespective of the direction, 0, in which the body is launched. 
For motion in a circle, e = 0. From (24) 

(30) - = 4 h 2 = MO. 
an 2 

Moreover, from (26) we see that = 7r/2, and so we infer from 
(27) that 

A 2 = via*. 

Hence, by the aid of (30), 

(31) v* = Jj. 

Conversely, conditions (30) and (31) are sufficient, that the 
path be a circle. For from (27) follows that cos 2 /3 = 0, and 
(29) gives 6 = 0. The result checks with the fact that the numer- 
ical value of R, or w/*/a 2 , is equal to the centripetal force, or 

EXERCISES 

1. Show that if 



then 



2 , , 

r 2 -rr = h and u = -, 
dt r' 



114 MECHANICS 

2. It has been assumed that the orbit is a plane curve. Prove 
this to be the case by means of a constraint, consisting of a smooth 
plane through 0, the point of projection, and the tangent to the 
path at that point. Use Newton's Equations, 17, (2), and 
show that the force of the constraint is 0. 

26. The Two Body Problem. If two particles of masses w, 
m'j attracting each other according to the law of nature, and 
acted on by no other forces, be projected in any manner, their 
centre of gravity, G, will describe a right line, with constant 
velocity, or remain permanently at rest ; cf. Chapter IV, 1. Con- 
sider the latter case. Let G be the fixed point 0, and let the 
distances of the particles from be r, r'. Then the force of their 
mutual attraction is 

/ = K ( r + r ')2> 

where K is the gravitational constant. On the other hand, 

mr = m'r'. 
Hence 

, _ m + m' 
r ~m' r ' 

and so 

' \2 



f m \ 2 , 
= ( - - - ,) m'. 
\m + ml 



Thus the particle m is attracted toward with the force that 
would be exerted by a mass M fixed at 0, and so the orbit of m 
is determined by the work of 25. In particular, if m describes 
an ellipse, m f will describe a similar ellipse with the same focus, 
being turned through an angle of 180. 

27. The Inverse Problem to Determine the Force. Let 

a particle move in a plane according to the Law of Areas. Then 

r^ = h 
T dt ft ' 

and the component of the force perpendicular to the radius vector, 
0, is nil. Hence the particle is acted on by a central force, R, 
either attractive or repulsive. From Exercise 1, 25, we have : 



MOTION OF A PARTICLE 115 

Example. Let the path be an ellipse (or, more generally, any 
conic) with the centre of force at a focus. Then 

1 e cos (07) , 

u = , p = const., 

P 

d*u . 1 

W* + U = p> 
and 

mh*l 
K ~ p r* 

The force is, therefore, an attractive force, inversely proportional 
to the square of the distance from the centre, when r lies between 
its extreme values for this ellipse. But an arbitrary range of 
values, < a < 7 < 0, can be included in such an ellipse, and so 
the result is general. 

EXERCISE 

Show that if the path is an ellipse with the centre of force at 
the centre, the force is proportional to the distance from the 
centre. 

28. Kepler's Laws. From observations made by Tycho 
Brahe, Kepler deduced the laws which govern the motion of 
the planets. 

1. The planets describe plane curves about the sun according 
to the law of areas; 

2. The curves are ellipses with the sun at a focus; 

3. The squares of the periodic times of revolution are proportional 
to the cubes of the major axes of the ellipses. 

Newton y s Inferences. From Kepler's laws Newton drew the 
following inferences. Consider a particular planet. From the 
first law it follows that the force acting on it is a central force, 
since the component at right angles to the radius vector is nil. 

From the second law, combined with the first, it follows from 
27 that the force is inversely proportional to the square of the 
distance from the centre, or 



116 MECHANICS 

It has been shown in 25, (21) that 

T2 = 47T 2 -, 
M 

where T denotes the periodic time, and a is the semi-axis major. 
For a second planet, 



Kepler's third law gives, then, that p! = p, or that /* is the same 
for all the planets. 

To sum up, then, Newton inferred that the planets are at- 
tracted toward the sun with a force proportional to their masses 
and inversely proportional to the square of their distances from 
the sun. 

From here it is but a step to the Law of Universal Gravita- 
tion. If the sun attracts the planets, so must, by the principal 
of action and reaction, the planets attract the sun. Let M denote 
the mass of the sun, thought of as at rest.* Then 



Thus the Law of Universal Gravitation is evolved : Any two 
bodies (particles) in the universe attract each other with a force 
proportional to their masses and inversely proportional to the 
square of the distance between them, or 



win 



The factor K is called the gravitational constant. Its value 
in c.g.s. units is 

# = 6.5X 10-*; 

cf. Appell, l.c., pp. 390-405. 

EXERCISES 

1. Show that the first of the equations (1), 25 : 



dt* dt 2 

* For a more detailed treatment cf. Appell, Mecanique rationnette, vol. 1, 3d ed., 
1909, 229 et seq. 



MOTION OF A PARTICLE 117 



on making the transformation (11) : 



. 

r* 
r dt 



and employing (2) : 

goes over into the equation : 

Hence obtain (16) : 

u = ~ + B cos (B 7). 

2. Prove that 

h 

v -, 
P 

where p denotes the distance from to the tangent to the path. 

3. Show that the earth's orbit, assumed circular, would 
become parabolic if half the sun's mass were suddenly annihilated, 
the sun being assumed to be at rest. 

4. A smooth tube revolves around one end in a fixed plane 
with constant angular velocity. A particle is free to move in 
the tube. Determine the motion. 

5. If, in the preceding question, an elastic string is made 
fast to the particle and attached to the end of the tube, deter- 
mine the motion. 

6. A particle is attracted toward a fixed centre with a force 
proportional to the distance. Show that the path is a plane 
curve, and that it can be represented by the equations : 

x = A cos (nt + a), y = B sin (nt + a). 

Is it an ellipse? 

7. Show that a comet describing a parabolic path cannot 

remain within the earth's orbit, assumed circular, for more than 

(2 \ 
- 1-th part of a year, or nearly 76 days. 

8. A shell is describing an elliptical orbit under a central 
attractive force. Prove that, if it explodes, all the pieces will 
meet again at the same moment ; and that after half the interval 
between the explosion and the collision, each piece will be moving 



118 MECHANICS 

with the same velocity as at the instant of explosion, but in the 
opposite direction. 

9. Show that a particle, moving under the action of a central 
force, cannot have more than two apsidal distances ; cf . Appendix B. 

10. Find the law of force when a particle describes a circle, 
the centre of force being situated on the circumference. 

Ans. The inverse fifth power. 

11. If two spheres, each one foot in diameter and of density 
equal to the mean density of the earth (5.6) were released from 
rest in interstellar space with their surfaces -^ inches apart, how 
long would it take them to come together? 

How great would the error be if their mutual attraction were 
taken as constant? 

12. A cannon ball is fired vertically upward from the Equator 
with a muzzle velocity of 1500 ft. a sec. How far west of the 
cannon would it fall, if the earth had no atmosphere ? 

13. Show that a particle acted on by a central repulsive force 
varying according to the inverse square, will in general describe 
a branch of a hyperbola with the centre of force at that focus 
which lies on the convex side of the branch. What is the excep- 
tional case? 

29. On the Notion of Mass. Matter is inert. It cannot exert 
a force; it cannot push or pull. It yields to force, acquiring 
velocity in the direction in which the force acts we are think- 
ing of a particle. By virtue of its inertness it possesses mass, 
which may be described as the quantity of matter which a body 
contains. 

Mass is measured by the effect which force produces on the 
motion of a body. We assume that force may be measured by 
a spring balance. If a force, constant in magnitude and direc- 
tion, be applied to a body initially at rest, the body will acquire 
a certain velocity in a given time. If the same force be applied 
to another body, and if the second body acquire the same veloc- 
ity in the same time, the two bodies shall be said to have the 
same mass. Thus different substances can be compared as to 
their masses and on adopting an arbitrary mass as the unit in 
the case of one substance, the unit can be determined in the 
case of other substances. 



MOTION OF A PARTICLE 119 

It was proved experimentally by Newton that the forces with 
which gravity attracts two masses equal according to the above 
definition, are equal. And so one is led to infer the physical 
law that the weight of a body is proportional to its mass. This 
law affords a convenient means of measuring masses, namely, 
by weighing. 

In abstract dynamics, however (to quote from Maxwell), 
matter is considered under no other aspect than that under which 
it can have its motion changed by the application of force. Hence 
any two bodies are of equal mass if equal forces applied to these 
bodies produce, in equal times, equal changes of velocity. This 
is the only definition of equal masses which can be admitted in 
dynamics, and it is applicable to all material bodies, whatever 
they may be made of.* 

In Engineering it has become customary to define masses as 
equal when their weights are equal. We have here a question 
of a sense of values, and Maxwell has gone on record as declaring 
unequivocally for the inertia property. To use weight to define 
mass is like saying that two lengths are equal when the rods by 
which we measure them have the same weight. Just as space 
and time stand above mass and force, so, in its elementary impor- 
tance, the inertia property towers above the law of gravitation. 

* Maxwell, Matter and Motion, Art. XL VI. 



CHAPTER IV 
DYNAMICS OF A RIGID BODY 

1. Motion of the Centre of Gravity. Let a system of particles 
be acted on by any forces whatever. The latter may be divided 
into two classes : i) the internal forces ; ii) the external forces. 
By i) we mean that the particle m z exerts on m 1 a force F 12 
which may have any magnitude and any direction whatever, 
or in particular not be present at all, F 12 = 0. The particle 
m l exerts a force on w 2 , which is denoted by F 2l . And now we 
assume the physical law that action and reaction are equal and 

opposite; i.e. that the vector F 21 
>2/2) is equal and opposite to the vec- 
tor F 12 , or 

Fi2 + F 21 = 0. 

FIG. 75 For convenience we will think of 

the particles and forces as lying in 

a plane. The transition to space of three dimensions is immediate. 
Denote the components of a vector force F along the axes of 
coordinates by X, Y. Then 

*i2 + X 21 = 0, F 12 + 7 21 = 0. 

Suppose there are three particles. Then Newton's Second Law 
of Motion gives for the first of them the equations : 

j. __ 




= X 1 + X n + X 1 



There are in all three such pairs of equations, those in x being the 
following : 

d*x d 2 x 



d 2 x 

~dfi = -^3 + 

120 



DYNAMICS OF A RIGID BODY 



121 



On adding these three equations together, the components 
Xu on the right, arising from the internal forces, annul one an- 
other in pairs, and only the sum of the Xi remains : 

a X\ . a Xn , Ci X-i -* r . *r r . 

m *~dP + m *~W + m *^W = Xl + X>2 + * 3 * 

In a similar manner we infer, by writing down the three equa- 
tions in y and adding, that 



m * "eft 2 ^ "^ "* 2 ^ft 2 ^ "^ "* 3 ~eft^ ~~ * * ^~ * ? ~"~ * 3 ' 

Precisely the same reasoning shows that if, instead of three, 
we have any number, n, of particles, the internal forces annul 
one another in pairs, and thus we obtain the result : 



Coordinates of the Centre of Mass. The left-hand sides of 
these equations admit a simple interpretation in terms of the 
motion of the centre of mass of the system. The coordinates, 
(x y y), of the centre of mass are given by the equations : 



(2) 



x = 



V = 



m n x n 2 



m n 
m n y n 



m 1 + + w n 
If we denote the total mass by M, then 

! rn k x k = 



Hence we have : 

d*x k 



a'Xk _ TUT- V 

~M ~ M ~jfLi 2* 



fc l*l/ H/w j^ 

and thus Equations (1) can be written in the form : 



(3) 



122 MECHANICS 

These equations are precisely Newton's Second Law of Motion 
for a particle of mass Af, acted on by the given external forces, 
each transferred to the particle. We can state the result as 
follows. 

THEOREM. The centre of mass of any system of particles moves 
as if all the mass were concentrated there and all the external forces 
acted there. 

In the case of particles in space, there is a third equation, 
(3) being superseded now by 



(4) * = ^ , . 

Remark. There is one detail in the statement of the theorem 
that requires explicit consideration. We have written down 
tbe differential equations of the motion, but we have not inte- 
grated them. If we do not start the particle of mass M in coin- 
cidence with the initial position of the centre of mass, it obvi- 
ously cannot describe the same path. More than this, we must 
give it the same initial velocity (i.e. vector velocity). Is this 
enough to insure its always remaining in coincidence with the 
centre of mass? The answer to this question is a categorical 
Yes ; cf. Chapter III, 17 and Appendix B. 

Generalized Theorem. We have proved the theorem of the 
motion of the centre of mass for a system of particles. In the 
case of a rigid body, we can think of the body as divided up into 
a large number of cells, each of small maximum diameter; the 
mass of each cell as then concentrated at one of its points, and 
the n particles thus resulting as connected by masslcss rods, 
after the manner of a truss.* To this auxiliary system of par- 
ticles the theorem as above developed applies. Arid now it is 
intuitionally evident, or plausible, that the system of particles 
will move in a manner closely similar to that of the rigid body, 
when the cells are taken very small. One is tempted to say 

* It is often necessary to use a truss, at some of whose vertices there are no 
masses. We may think of minute masses attached at these points and acted on 
by gravity or by no external forces at all. The effect of these small masses is to 
modify slightly the value of M in Equations (4). And now it follows from the 
theory of differential equations that the integrals of (4) are thereby also modified 
only slightly. Hence the physical assumption is made, that Equations (4) hold 
even when there are no masses at the vertices in question. 



DYNAMICS OF A RIGID BODY 123 

that the motion of the actual body is the limit approached by 
the motion of the system of particles as n grows large and the 
cells small. And this is, in fact, true. But this is not a mathe- 
matical inference far from it it is a new physical postulate. 
We thus extend the theorem and elevate it to a Principle.* 

PRINCIPLE OF THE MOTION OF THE CENTRE OF MASS. The 
centre of mass of any material system whatsoever moves as if all the 
mass were concentrated there, and all the external forces acted there : 



A) 



2. Applications. The Glass of Water. Suppose a glass of 
water is thrown out of a third-story window. As the water falls, 
it takes on most irregular forms, breaking first into large pieces, 
and these into smaller ones. The forces that act are gravity 
and the resistance of the atmosphere, the latter spread out all 
over the surfaces of the pieces. And now the Principle of the 
last paragraph tells us that the centre of gravity moves as if 
all the mass were concentrated there and all these forces trans- 
ferred bodily (i.e. as vectors) to that point. 

The Falling Chain. Let a chain hang at rest, the lower end 
just touching a tablo, and let it be released. To determine the 
pressure, F, on the table. 

We idealize the chain as a uniform flexible string, of length / 
and density p (hence of mass M = pi), and think of it as im- 
pinging always at the same fixed point, 0, of the table. Let s 
be the distance the chain has fallen and let x be the height of 
the centre of gravity above the table. Then the Principle of 
the Motion of the Centre of Mass gives the equation : 

* A "Principle" in Mechanics is well described in the words of Professor Koop- 
nrian (of. the Author's Advanced Calculus, p. 430): "According to the usage of 
the present day the word principle in physics has lost its metaphysical implication, 
and now denotes a physical truth of a certain importance and generality. Like 
all physical truths, it rests ultimately on experiment ; but whether it is taken as a 
physical law, or appears as a consequence of physical laws already laid down, 
does not matter." 



124 



MECHANICS 



(1) 



Now, 



~ a ' 

s - ld*s I 



G * 

' Opl 



I dt*' 



Moreover, from the laws of freely falling 
bodies, 



Fia. 76 



On substituting those values in (1), we 
obtain : 



(2) 

Hence 

(3) 



OP (s - 1) + 



F - gpl. 



or 



F = gps + pv 2 , 
F = 3gps. 



This means that the pressure of the chain on the table is always 
just three times the weight of that part of the chain which has 
already come to rest on the table. 

It appears, then, that F is made up of two parts, i) the pres- 
sure gps on the table, of that part of the chain already at rest; 
and ii) a pressure 

(4) P = pv*, 

due to the impact of the chain against the table. 

A Stream of Water, Impinging on a Wall. Suppose a hose is 
turned on a wall (or a convict !). To determine the pressure. 

We idealize the motion by thinking of the stream as hitting 
the wall at right angles, the water spattering in all directions 
along the wall and thus giving up all its velocity in the line of 
motion of the stream. 

Dynamically, this is precisely the same 
case as that of the chain falling on the table, 
so far as the impact is concerned, and hence 
the pressure is given by (4) : FIG. 77 

PA 
== ov * 




DYNAMICS OF A RIGID BODY 125 

Example. A fire engine is able to send a 2 in. stream to a 
vertical height of 200 ft. Find the pressure if the stream is 
played directly on a door. Ans. 541 Ibs. 

The Crew on the River. The crew is out for practice. Ob- 
serve the cut-water of the shell and describe how it moves, and 
why it moves as it does. What system do you decide to isolate ? 
the shell? or the shell, oars, and crew? 

EXERCISES 

1. If a man were placed on a perfectly smooth table, how 
could he get off? 

2. If a shell were fired from a gun on the moon and exploded 
in its flight, what could yo.u say about the motion of the pieces ? 

3. A goose is nailed up in an air tight box which rests on plat- 
form scales. The goose flies up. Will the scales register more or 
less or the same? 

4. A pail filled with water is placed on some scales. A cork 
is held submerged by a string tied to the bottom of the pail. 
The string breaks. Do the scales register more or less or the 
same? 

6. A man, standing in the stern of a row boat at rest, walks 
forward to the prow. What can you say about the motion of 
the boat? 

6. When the man stops at the prow of the boat, boat and man 
will be moving forward with a small velocity. Explain why. 

7. A uniform flexible heavy string is laid over a smooth 
cylinder, axis horizontal, and kept from slipping by holding 
one end, A, fast, the part of the string from A up to the cylinder 
being vertical. The part of the string on the other side of the 
cylinder is, of course, also vertical, its lower end, /?, being below 
the level of A, and the whole string lies in a vertical plane per- 
pendicular to the axis of the cylinder. The string is released 
from rest. Determine the motion, there being a smooth guard 
which prevents the string from leaving the upper side of the 
cylinder. 

8. If, in Question 7, the difference in level between A and 
R is 2 ft., and if the distance from A up to the cylinder is 8 ft., 



126 



MECHANICS 



compute the velocity of the string when the upper end reaches 
the cylinder, correct to three significant figures. 

9. Find how long it takes the upper end of the string to reach 
the cylinder. 

10. The sporting editor of a leading newspaper recently re- 
ported a new stroke which a certain coach had developed, the 
advantage of which was that it gave an even motion to the shell 
and avoided the jerkiness 01 the old-fashioned strokes. Examine 
this news item. 

3. The Equation of Moments. Recall the formula for the 

moment of a force F about the origin, 
namely, 

(1) xY-yX. 

Consider a system of particles acted 

on by any external forces whatever, 

and interacting on one another by 
forces that are equal and opposite, but 
are now assumed each time to lie in the lino joining the two par- 
ticles in question. Moreover, the particles shall lie in a fixed 
plane. Begin with the case of 
three particles, as in 1, and 
write down the six equations that 
express Newton's Second Law 
of Motion for these particles.* 
Next, form the expression : 




FIG. 78 



FIG. 79 



m l 



r 



and compute its value from the equations in question, namely, 
(x, Y l - Vl X,) + (x, Y 12 - Vl X 12 ) '+ (x, Y n - y, X n ). 

The parentheses represent respectively the moments of F D F 12 , 
F 13 about the origin. 

Now, do the same thing for the particle ra 2 , and finally, for ra 3 . 
On adding these three equations together, it is seen that the 

* It is important that the student do this, and do it neatly, and not merely gaze 
at the three equations printed in 1 and try to imagine the three not printed. 
He should write out the full equation derived below from these, neatly on a single 
line, and then write the other two under this one. 



DYNAMICS OF A RIGID BODY 



127 



moments of the internal forces about the origin destroy one 
another, and there remains on the right-hand side only the sum 
of the moments of the applied forces. 

If there are n > 3 particles, m lt w 2 , , m n , the procedure is 
the same, and we are thus led to the 



THEOREM OF MOMENTS: 



B) 



m k 



d*Xk 



- yA). 



We refrain from writing down the corresponding theorem in 
three dimensions, because we shall have no need of it for the 
present. 

4. Rotation about a Fixed Axis under Gravity. Let the 

system of particles of 3 be rigidly connected, and let one point, 
O, of the trass-work be at rest, so that the system rotates about 
as a pivot. For example, take the case of a uniform rod, one 
end of which is held fast, and which is released from rest under 
gravity. Divide the rod into n equal parts, x 
and concentrate the mass of each part, for defi- 
niteness, at its most remote point. We thus 
have a system of n particles, and we connect 
them rigidly by a massless truss-work as shown 
in the figure.* 

We are now ready to compute each side of 
Equation B) for the auxiliary system of n par- 
ticles. Let r be the distance from to any 
point fixed in the rod. Then 

(1) x = r cos 0, y = r sin 0, 

where varies with the time, t, but r is constant with respect 
to t. Hence 




Fia. 80 



(2) 



dx . _ dO 

-rr = T Sill -7T, 

dt dt 



$-- 



We observe next that, in all generality, by mere differentia- 
tion, i.e. purely mathematically, 



(3) 



<L ( d-i 4*\ - d*y _ 

di\ x ~di y dt)~ x d? 



* Cf. the footnote, I. 



128 MECHANICS 

and we proceed to compute the parenthesis by means of Equa- 
tions (1) and (2). We find : 

dy dx ~dO 



In the present case we have : 

d ( dy k dx k \ _ d*8 

dt\ Xk dt yk ~dt) -~ rt ~dT 

for r k does not change with the time, and so dr k /dt = 0. Hence 



The sum which here appears is the moment of inertia* of the 
system about : 



Thus the left-hand side of the Equation of Moments reduces to 
the expression : 



Turning now to the right-hand side of B) we see that the 
k th particle, m/t, yields a moment about equal to the quantity 
m k gr k sin 0, and so the sum in question becomes 

] - m k gr k sin 0, or - (2) m k rk)g sin 0. 

t t 

But m k r k = Mh y 



where h is the distance from to the centre of gravity, (?, of the 
system of particles. Hence, finally, 

(6) I^ 2 =-MghsmO. 

This is substantially the equation of Simple Pendulum Motion, 
Chapter III, 20 : 

^\ d 2 6 g . . 



* Moments of inertia for such bodies as interest us here are treated in the 
Author's Introduction to the Calculus, p. 323. 



DYNAMICS OF A RIGID BODY 129 

Hence the system of n particles oscillates like a simple pendulum 
of length 

l = m 

or 

(8 2 ) I = j, where 7 = M W, 

k denoting the radius of gyration. 

More precisely, what we mean by the last statement is this. 
Let a simple pendulum be supported at 0, let its length be k*/h, 
and let it be placed alongside the rod, the bob being at a point 
distant Z from O. If now both be released from rest at the same 
instant, they will oscillate side by side, though not touching each 
other. 

The Actual Rod. As n grows larger and larger, the massless 
rod weighted with the n particles comes nearer and nearer to 
the actual rod, dynamically. This is not a mathematical state- 
ment. It expresses our feeling from physics for the situation 
our intuition. And so whon we say that the motion of the actual 
rod is the limit approached by the motion of the auxiliary rod, 
we are stating a new physical postulate. The result is, that the 
actual rod oscillates like a simple pendulum of length 

fc_ 2 -iL 2 -?/ 
h # 3 

EXERCISES 

Apply the method set forth in the text, introducing each time 
an auxiliary set of particles, and proceeding to the limit. Do 
not try short cuts by attempting to use in part the result of the 
exercise worked in the text. 

1. A rod 10 ft. long and weighing 30 Ibs. carries a 20 Ib. weight 
at one end and a 30 Ib. weight at the other. It is supported 
at its middle point. Find the length of the equivalent simple 
pendulum. Ans. 30 ft. 

2. Equal masses are fixed at the vertices of an equilateral 
triangle and the latter is supported at one of the vertices. If it 
be allowed to oscillate in a vertical plane, find the length of the 
equivalent simple pendulum. 



130 



MECHANICS 



3. A rigid uniform circular wire * 6 in. in diameter and weigh- 
ing 12 Ibs. has a 4 Ib. weight fastened at one of its points and 
is free to oscillate about its centre in its own plane. Find the 
length of the equivalent simple pendulum. 

4. Equal particles are placed at the vertices of a regular hexa- 
gon and connected rigidly by a weightless truss. The system 
is pivoted at one of the particles and allowed to oscillate in a 
vertical plane under gravity. Find the length of the equivalent 
simple pendulum. 

6. Generalize to the case of n equal particles placed at the 
vertices of a regular n-gon. 

6. The Compound Pendulum. Consider an arbitrary lamina, 
or plane plate of variable density. Let it be supported at a 
point arid allowed to oscillate freely in its own plane, assumed 
vertical, under gravity. This is essentially the most general 
compound pendulum. To determine the motion. 

Divide the lamina up in any convenient manner into small 
pieces and concentrate the mass of each piece at one of its points. 

Connect these particles with one 
another and with the support at 
by a truss-work. The auxiliary sys- 
tem can be dealt with by the Prin- 
ciple of Moments. Set 




%k ^k COS 6k, 

Then 



y k = r k sin 0*. 



FIG. 81 



Now, draw a line in the lamina, 
for example, the line through and 
the centre of gravity, G, of the 

particles, and denote the angle it makes with the axis of x by 0. 

Then 



where ct k varies with fc, but is constant as regards the time. Hence 

d0k = de d 2 B k = d*0 

dt " dt' dP ~~ dt* 



* By a wire is always meant a material curve. 



DYNAMICS OF A RIGID BODY 131 

Thus the left-hand side of the Equation of Moments, 3, 
becomes 

n\ V 1& T dze 

(1) ? m * r *^ = / ^> 

where 7 denotes the moment of inertia of the system of particles 
about 0. 

The right-hand side of B), 3, can be written 

(2) 2) " m kgyk = -02) m ky*' 

The last sum has the value My, whore the coordinates of G 
are denoted by (x, y). Let the distance from to G be h. Then 

y = h sin 
and (2) becomes 

(3) - M0/i sin 6. 

On equating (1) and (3) to each other, we have 

d~n 

(4) /5y[=- JfffAsinfl. 

This is the Equation of Simple Pendulum Motion, and 



It appears, then, that the auxiliary system of particles oscillates 
like a simple pendulum. As we allow n to increase without limit, 
the maximum diameter of the little pieces approaching 0, it seems 
plausible that the motion will approximate more and more closely 
to that of the actual compound pendulum, and this consider- 
ation leads us to lay down the physical law, or postulate, that 
Equation (4) holds for the compound pendulum, where 7 and 
h now refer to the latter body. 

Remark. We have thought of the mass of the compound 
pendulum as two-dimensional, or lying in a plane. But this is 
obviously an unnecessary restriction. Conceive a block of 
granite, blasted from the quarry as irregular and jagged as 
you please. Mount it on two knife-edges, so it can swing about 
a horizontal axis. Now this block will obviously oscillate exactly 
as a plane lamina perpendicular to the axis would, if the mass 
of the actual block were projected parallel to the axis on a plane 
at right angles to the axis. 



132 MECHANICS 

The above "obviously" is not to be taken mathematically, 
but is a new physical law, or postulate. It is true that when 
we come to treat the general case of motion in three dimensions, 
this postulate will be merged in more general ones. 

EXERCISES 

Find the length of the equivalent simple pendulum when the 
compound pendulum is one of the following. 

1. A uniform circular disc, free to rotate in its own plane 
about a point in its circumference. Ans. I = f r. 

2. A circular wire, about a point of the wire. Ans. I = 2r. 

3. Question 1, when the axis is tangent to the disc. 

Ans. I = fr. 

4. Question 2, when the axis is tangent to the wire. 

Ans. I = -Jr. 
6. A rectangular lamina, about a side. 

6. A square lamina, about a vertex. 

7. A triangle, about a vertex. 

6. Continuation. Discussion of the Point of Support. Let 

7 = Mfc 2 

be the moment of inertia of the compound pendulum about a 
parallel axis through the centre of gravity, (?. By the theorem 
of 10 the moment of inertia about the actual axis will be : 



and the length of the equivalent simple pendulum is soon from 
(5), 5, to be : 

(6) I = ^A 2 - 

The question arises: What other points of support, (i.e. 
what other parallel axes), yield the same period of oscillation? 

Clearly they are those, and only those, whose distance, x, 
from satisfies the equation, 

,_* + * 



x 
(7) x* - Ix + Jk 2 = 0, 



DYNAMICS OF A RIGID BODY 



133 



where k and I are given, and where, more- 
over, (6) is true, or 

(8) h* - Ih + k 2 = 0. 

One root of Equation (7) is x l = h. 
The other is seen to be 

_i j, _ * 2 
^ - I - ft _ ~ 

We can state the result as a theorem. 




FIG. 82 



THEOREM. The locus of the points 0, for which the time of oscil- 
lation is the same y consists of two concentric circles with their centre 
at G, their radii being 

, , k 2 
h and -r- 
fi 

EXERCISES 

1. Draw two concentric circles about G, of radii h and k*/h. 
Show that the length, Z, of the equivalent simple pendulum cor- 
responding to an axis through a point on one of these circles 
is obtained by drawing a line from through G, and terminating 
it whore it meets the other circle. 

This theorem is due to Huygens. 

2. Show that the locus of the points of support, for which 
the time of oscillation is least, form a circle with G as centre and 
of radius k. 

7. Kater's Pendulum. The experiment for determining the 
value of g, the acceleration of gravity, by means of a simple 
pendulum and the formula 

T = 

9 

is familiar to all students of physics and mathematics. The 
chief error in the result arises from the error in determining I. 
The bob is not sensibly a particle and the string stretches. 

To attain greater accuracy, Kater made use of Huygens's 
Theorem, 6, Ex.1, constructing a compound pendulum that 
could be reversed. It consists essentially of a massive rod, 
or bar, provided with two sets of adjustable knife-edges. These 
edges lie in two parallel lines, and the centre of gravity, (?, is 



134 MECHANICS 

situated in their plane, at unequal distances, h and A', from them. 
The knife-edges are now so adjusted experimentally that the 
period when the pendulum oscillates about the one pair is the 
same as when it is reversed and allowed to oscillate about the 
other pair. Since 

I = h + h', 

the determination of the length of the equivalent simple pendulum 
can now be made with great accuracy by measuring the distance 
between the knife-edges. Indeed, the accuracy in thus deter- 
mining g is now so great that very small errors, like those due 
to the buoyancy of the air, the changes in the pendulum due to 
changes in temperature, and the give of the supports have to 
be considered. For an elaborate and interesting account, cf. 
Routh, Elementary Rigid Dynamics, 98 et seq. 

8. Atwood's Machine. An Atwood's Machine consists of a 
pulley free to rotate about a horizontal axis, and a string passing 
over the pulley and carrying weights, M and M + m, at its two 
ends. It may be used to measure the acceleration of gravity. 

Our problem is to determine the motion of the system. The 
"system" which we choose to isolate is the complete system 
of pulley and weights, the mass of the string being assumed 
negligible. This is not a rigid system, but still, if we replace 
the pulley by a system of particles rigidly connected, the internal 
forces of the complete auxiliary system will satisfy the hypothesis * 
of 3, and thus the Equation of Moments will hold. 

For the auxiliary system of particles due to the wheel the 
contribution to the left-hand side of the Equation of Moments, 
B), 3, becomes as in the case of the compound pendulum : 



where I denotes the moment of inertia of this system about the 
axis, and B is the angle through which the wheel has rotated. 

* Consider a short interval of time in the duration of the motion. In the 
auxiliary system, let each vertical segment of the string be fastened to a particle 
near the point of taiigericy of the string in the actual case. Then it is plausible 
physically that the motion of the auxiliary system during this short interval differs 
but slightly from that of the actual system. Hence we may assume that the force 
of the string always acts at the points of tangency with the wheel, and neglect the 
rest of the string which is in contact with the wheel. But this is a new physical law. 



DYNAMICS OF A RIGID BODY 



135 



Let the radius of the wheel (more precisely, of the groove in 
which the string lies) be a. Observe, too, that 



y l = const. + a0, 



= const. aO. 




Thus the remaining contributions to the left- 
hand side of B), 3, will be 

(2) (M + m) a 2 -^ + Ma 2 -^ 

The right-hand side of B) reduces to 

(3) (M + m) ga Mga = mga. 
Thus B) becomes : 

dt 2 



This, for the auxiliary system of particles. And now we assume, 
physically, that the limit approached by the motion of the auxiliary 
system is the motion of the actual system ; i.e. that Equation (4) 
holds for the actual system. 

Let s denote the distance the weight and rider have descended. 
Then s = aO, and from (4) it follows that 



(5) 



mga' 



dt 2 I + (2M + m) a 2 
On integrating this equation we have, in particular, that 



(6) 



s = 



I + (2M + m) a 2 



Corresponding values of s and t can be observed experimentally. 
Thus Equation (6) is equivalent to a linear equation in the two 
unknowns, //a 2 and g : 



~ 

II 



0. 



If M is held fast and m is given different values, it is clear that the 
coefficient of g will take on different values, and so we shall have 
two independent linear equations for determining the unknown 
physical constants, 7/a 2 and g. 



136 MECHANICS 

EXERCISES 

In working these exercises use the method, not the result, of 
the text. Begin each time by drawing a figure. 

1. Suppose that the wheel is a uniform circular disc weighing 
10 Ibs., and that 5 Ib. weights are fastened to the two ends of 
the string. What will be the acceleration due to a 1 oz. rider? 

2. Work the case in which the wheel is a hoop, i.e. a uniform 
circular wire, the masses of the spokes being negligible; and 
show that the acceleration of the rider does not depend on the 
radius, but only on the mass of the hoop, and M and m. 

3. Determine the tensions in the string in the general case. 

4. Find the reaction on the axis. 

6. Prove the assertion in the text about the coefficient of g's 
taking on different values when m is varied. 

6.* How rough must the string be in the general case, in order 
not to slip? 

9. The General Case of Rotation about a Point. Consider 
an arbitrary rigid body in two dimensions, acted on by any forces 
in its plane, and free to rotate about a point 0, i.e. about an 
axis through perpendicular to the plane. Then, I say, its 
motion is determined by the Principle of Moments, 

B) / -jT2 = 5J Moments about 0. 



The Principle is rendered plausible by dividing the actual 
distribution into small pieces, as in the example of the corn- 
pound pendulum and the Atwood's machine, and observing that 
the Principle is true for the auxiliary system. The limit ap- 
proached by the motion of the auxiliary system is the motion 
defined by Equation B) of the present paragraph. And thus we 
are led to lay down the physical postulate that this is the motion 
of the actual system. Equation B), then, is an independent 
physical law, made plausible by the mathematical considerations 
set forth above, but not following mathematically from them. 

The Effect of Gravity. Whenever gravity acts, the contribu- 
tion of this force to the right-hand side of Equation B) can 

* This problem is more difficult than the others, and is essentially a problem in 
the Calculus ; cf. the author's Advanced Calculus, Chapter 14, 8. 



DYNAMICS OF A RIGID BODY 137 

always be written as the moment of a single force, that force 
being the attraction of gravity on a single particle of mass equal 
to the mass of the entire body and situated at the centre of gravity 
of the body. This is true in the most general case of motion, 
when no point of the body is permanently at rest. Here, again, 
we have a new physical postulate. 

EXERCISES 

1. A turn table consisting of a uniform circular disc is free 
to rotate without friction about its centre. A man walks along 
the rim of the table. Find the ratio of the angle turned through 
by the table to the angle described by the man, if man and table 
start from rest. 

2. The same problem when the man walks in along a radius 
of the table, the system not being, however, initially at rest. 

10. Moments of Inertia. The moment of inertia of the 
simpler and more importanjb distributions of matter are deter- 
mined by the methods of the Integral Calculus ; cf. for example 
the author's Introduction to the Calculus, p. 323, and the Advanced 
Calculus, pp. 58, 79, 88. 

Ml 2 

1. A uniform * rod of length I about one end : 5 

o 

TI/T 2 

2. A rod of length 2a about its midpoint : $ 



3. A circular disc about its centre : 5 

& 

Mr 2 

4. A circular disc about a diameter : ~T~~' 

5. A square about its centre : f M a 2 . 

6. A square about a side; cf. Example 1. 

7. A scalene triangle about a side : , 
where h denotes the altitude. 

o A i i * r * 

8. A sphere about a diameter : 

9. A cube about a line through the centre parallel to an edge ; 
cf. Example 5. 

* It will henceforth be understood that the distribution is uniform unless the 
contrary is stated. 



138 MECHANICS 

A GENERAL THEOREM. The moment of inertia of any distribu- 
tion of matter whatever, about an arbitrary axis, is equal to the mo- 
ment of inertia about a parallel axis through the centre of gravity, 
increased by Mh 2 : 



where h denotes the distance between the axes. 

We will begin by proving the theorem for a system of particles. 
Let the first axis be taken as the axis of z in a system of Cartesian 
coordinates, (x, y, z) ; and let the second axis be the axis of z' 
in a system of parallel axes. Then 

/ = 2 m k (x,? + 2/* 2 ), 7 = 2 w* W + yi 2 ). 

Since 

x = x' + x, y = y' + y, 
it follows that 



) = 2 

k . 

2x m k xi + 2y <k yi- 



The last two terms vanish because 0' is the centre of gravity, 
and hence 

2 m k x't = o, 2 



It remains merely to interpret the terms that are left, and 
thus the theorem is proved for a system of particles. 

If we have a body consisting of a continuous distribution of 
matter, we divide it up into small pieces, concentrate the mass 
of each piece at its centre of gravity, form the above sums, 
and take their limits. We shall have as before 2mkX r t = 0, 
S mk yi = 0, and hence 



lim 2 *(** 2 + 2/t 2 ) = Km 

n-oo j7 n = oc 



or 



since these limits are by definition the moments of inertia for the 
continuous distribution. 



DYNAMICS OF A RIGID BODY 139 

Example. To find the moment of inertia of a uniform cir- 
cular disc about a point in its circumference. Here, 7 = %Mr 2 

and h = r. Hence T Q ,. , 

/ = f Mr 2 . 

11. The Torsion Pendulum. Let a rod be clamped at its 
mid-point to a steel wire and suspended, the rod horizontal and 
the wire vertical. Let the rod be displaced slightly in its hori- 
zontal plane, the wire remaining vertical, arid then released. To 
determine the motion. 

The forces acting on the rod amount to a couple, due to the 
torsion of the wire, and the moment of the couple is propor- 
tional to the angle through which the rod is displaced such 
is the law of elasticity. Thus the Principle of Moments, 9, 
yields in this case the differential equation, 



Ma 2 
where / = ^ is the moment of inertia of the rod, and K is the 

constant of the wire. 

Equation (1) is the equation of Simple Harmonic Motion, 
and thus the period of oscillation, 



(2) T = 2* 

is the same, no matter what the initial displacement may have 
been, provided merely that the distortion of the wire is not so 
great as to impair the physical law above stated, and provided 
damping is neglected. 

12. Rotation of a Plane Lamina, No Point Fixed. Let a rigid 
plane lamina be acted on by any forces in its plane, and let it 
move in its plane. To determine the motion. 

The centre of gravity will move as if all the mass were con- 
centrated there and all the forces were transferred to that point ; 
1. It remains to consider the rotation. 

PRINCIPLE OF MOMENTS. The lamina rotates as if the centre 
of gravity were held fast and the same forces acted on the lamina as 
those applied in the actual case y 

(1) ^"77/2 = S Moments about (?, 



140 MECHANICS 

where I denotes the moment of inertia about the centre of gravity, G; 
6 is the angle that a line fixed in the lamina makes with a line fixed 
in the plane, and the right-hand side is the sum of the moments of 
the forces about G. 

Proof. Consider first a system of particles rigidly connected. 
Let (x, y) be axes fixed in the plane, and ( , 77) parallel axes whose 
origin is at G. Then 

(2) x = + a, y = 77 + y, 

and 



the omitted terms vanishing for the reason that 

>k * = 0, ] m k rj k = 0, 
and hence, too, 



Remembering that 



dt\dt 
we see that Equation B), 3, here becomes : 



Because 

x k = & + x, y k = ri k + y, 

the right-hand side of Equation (4) becomes : 

2 fen - rjkXk) + 
7 
Since 



DYNAMICS OF A RIGID BODY 141 

it follows that 



On subtracting this equation from (4), there remains : 
(5) * 



In this equation is contained the proof of the theorem for a 
system of n particles. For, the left-hand side reduces to the 
left-hand side of (1), since the distance of the point (&, ?/*) from 
the centre of gravity, G, does not change with t; and the right- 
hand side expresses precisely the sum of the moments of the 
applied forces about G. 

Finally, we pass to a continuous distribution of matter in 
the usual way, laying down a new physical postulate to the effect 
that Equation (1) shall hold for all rigid distributions of matter 
in a plane. 

13. Examples. A hoop* rolls down a rough inclined plane 
without slipping. Determine the motion. 

The forces are: the force of gravity and the reaction of the 
plane. Let the latter force be resolved into a normal com- 
ponent, R, and the tangential force of fric- 
tion, F, acting up the plane. Then, for 
the motion of the centre of gravity, we shall 
have: 




-. FIQ 84 

The second equation for the motion of the centre of gravity 
merely tells us that 

(2) R = M g cos a, 

a fact that we could have guessed, since the centre of gravity 
always remains at the same distance from the plane. However, 
let us formulate the second equation, and prove our guess right. 
Let y denote the distance of the centre of gravity from the plane. 

* A pipe, the thickness of which is negligible, when placed on the plane with its 
axis horizontal, would move in the same way. The two problems are dynamically 
identical. 



142 MECHANICS 

Then 

But y = a, the radius of the hoop, and so the left-hand side of 
this equation is 0. 

Turning now to the rotation of the hoop, we write down Equa- 
tion (1) of the Theorem, 12 : 

(4) /-^ = aF, I = Ma 2 . 

Since there is no slipping, 

(5) 5 = a0, 

where, for convenience, we take as 6 the angle that the radius 
drawn to the point of contact with the plane at the start has 
turned through, 5 being also at the start. 
Equations (1) and (4) can now be written in the form : 

Ma -JTJ = Mg sin a F, 
(6) 

Ma*<^ = aF. 

On eliminating F between these equations, we find : 

or 

(8) ^ = | sina . 

Hence it appears that the centre of the hoop moves down the 
plane with just half the acceleration it would have if the plane 
were smooth. 

Equation (2) appears to have played no part in the solution. 
But we have assumed that there is no slipping, and so F cannot 
be greater than pR : 

(9) F ^ R. 

To ascertain what this condition means for the coefficient 
of friction, ju, and the steepness of the plane, a, solve Equations 

(6) for F and substitute : 

F ^y s * n a 

2 ' 



DYNAMICS OF A RIGID BODY 143 

Mg sin a . . 

2-5 ^ M^ cos a, 

(10) tan a ^ 2 M . 

Hence it appears that a may not exceed tan" 1 2ju. 

EXERCISES 

1. Show that, if the hoop be released from rest, 

gt . at* . 

v = ~ sm a, s = ~- sm a, 

v 2 = 0s sin a. 

2. Show furthermore that 

at . at 2 . 

= TJ- sin a, ^ = T- sin a, 

<&& 4<z 

W 2 *L gj n a 

a 

3. Solve the problem studied in the text for a sphere. Show 
that 

d*6 5g . d*s 50 . 

^5 = ^ am a, ^J^Bina. 

4. Prove that the sphere will slip unless 

tan a g JJLI. 
6. Make a complete study of a disc, or solid cylinder. 

14. Billiard Ball, Struck Full. A billiard ball is struck full 
by the cue. To determine the motion. 

The forces are: the force of gravity, acting downward at the 
centre of gravity, and the reaction of the billiard table, which 
yields a vertical component, R, and a horizontal component, F. 
Let s be the space described by the centre of the ball, and 6, the 
angle through which the ball has turned.* 

The Principle of the Motion of the Centre of Gravity, 1, 
yields the equations : 



(1) 




__ 

dt* 

F 

R = Mg FIG. 85 



* It is of prime importance that the student begin each new problem, as here, 
by drawing a figure showing the forces and the coordinates used in setting up the 
differential equations of the motion. It is well, too, to note at the same time any 
auxiliary relations, as in the present instance, F = pR. 



144 MECHANICS 

The Principle of Rotation about the Centre of Mass, 12, 
yields the equation : 

tv\ r d * e nw T 

(2) 7 = ^ I 



Finally, so long as there is slipping, 
(3) F = MB. 

From Equations (1), (2), and (3) it appears that 

/A \ &S 

(4.) i s= - r ' 



d< 2 ~ 2a 

The integrals of these equations are as follows : 
,g . f v = v - ngt, s = v t- 

\ t> 2 = vl - 

and 



Thus as the ball advances, its centre moves more and more 
slowly, while the speed of rotation steadily increases. Finally, 
pure rolling will set in. This takes place when the velocity of 
the point of the ball in contact with the table is nil. Now, the 
velocity of this point of the ball is made up of two velocities, 
namely, i) the velocity of translation, or the velocity the point 
would have if the ball were not rotating, i.e. v, as given by (50; 
and ii) the velocity due to rotation, or the velocity the point 
would have if the ball were spinning about its centre, thought of 
as at rest. The latter is a velocity of ao> in the direction opposite 
to the motion of the centre, and is given by (5 2 ). Thus the ve- 
locity forward of the point of the ball in contact with the table is 

(6) v ow. 

Slipping continues so long as this expression is positive, and 
ceases when it vanishes : 

(7) v oo> = 0. 



DYNAMICS OF A RIGID BODY 145 

The time is given by the equation 



or 



The corresponding value of s is seen to be : 



The angle through which the ball turns is 



Finally, 

(11) 1 = |>0, ! = T 2 ' 

7 la 

EXERCISES 

1. Solve the same problem in case the table is slightly tipped 
and the ball is projected straight down the plane. 

2. Work the last problem with the modification that the ball 
is projected straight up the plane. 

15. Continuation. The Subsequent Motion. At the end of 

the stage of the motion just discussed, the ball has both a mo- 
tion of translation and one of rotation, the point of the ball 
in contact with the table being at rest. If from now on the force 
exerted by the table on the ball consists solely of an upward 
component R and a tangential component F, the latter force will 
vanish, and the ball will continue to roll without slipping. For, 
suppose the table is rough enough to prevent slipping. Then 
s = oQ, and since equations (1) and (2) still hold, we have : 

Hence F vanishes, and the angular and linear accelerations are 
both 0, too. 

But in practice the ball will slow up. How is this to be ac- 
counted for, if the resistance of the air is negligible? The answer 
is, that the reaction of the table is not merely a force, with com- 
ponents R and F. but, in addition, a couplej the moment of which 



146 MECHANICS 

we will denote by C. This couple has no influence on the motion 
of the centre of gravity; thus Equations (1), 14, remain as 
before. But Equation (2) now becomes 



O 



(13) 



FIG. 86 Furthermore, 
(14) 
Hence 



dP 7 Ma' dt* 7 Ma*' la 

Since C is small, the ball slows up gradually. 

EXERCISES 

1. If the centre of the ball was moving initially at the rate of 
6 ft. a sec. and if the ball stops after rolling 18 ft., show that 

C = IMa. 

2. If the initial velocity of the centre was V Q and if the ball 
rolled I ft., show that C is proportional to the initial kinetic energy 
and inversely proportional to the distance rolled. 

16. Further Examples, i) HOOP ON ROUGH STEEPLY IN- 
CLINED PLANE. Suppose, in the Example studied in the text 
of 13, that a does exceed tan" 1 2/*. What will the motion then 
be, the hoop being released from rest? 

Equations (1), (2), and (4) will be as before. But now (5) is 
replaced by the equation : 

(i) p = & 

all the friction now being called into play. On eliminating P 
and R, we find : 



(2) 



d z s 

- = <7(sin<* - 



-= = cos a. 
dt 2 a 



The integrals of these differential equations can be written 
down at once. In particular, it is seen that the ratio of s to 6 
is constant, if the hoop starts from rest : 

s a (sin a u cos a) ,, , % -, 

- = - - - '- = o(tan a cot X - 1). 
p cos a 



DYNAMICS OF A RIGID BODY 



147 




FIG. 87 



The last parenthesis has the value 1 when tan a = 2/z, and 
is > 1 when a is larger. Thus the motion is one in which a cir- 
cle of radius , _ 

r = a (tan a cot X 1) 

and centre at the centre of the hoop rolls 

without slipping on a line parallel to the 

plane and beneath it. We have here an 

illustration of the general theorem that any 

motion of a lamina in its own plane can be 

realized by the rolling without slipping of a curve drawn in the 

lamina on a curve drawn in the plane ; cf. Chapter V, 4. 

ii) LADDER SLIDING DOWN A SMOOTH WALL. First, draw a 
figure representing the forces and the coordinates. 
The three equations of motion thus become : 



(3) 




FIG. 88 



"77/2 = a ^ s * n "~ a ^ cos ^ ^ = 

U/t" 



With these three Dynamical Equations are associated two 
Geometrical Equations : 

(4) x = a cos 0, y = a sin 6. 

These five equations determine the five unknown functions x, y, 
0, R, S, the time being the independent variable ; or they deter- 
mine five of the variables x, y, 0, R, /S, t as functions of the 
sixth. Eliminate 72, S between the first three equations: 



< 5 > '.- 



> -^ M a cos ~ Af gra cos 6. 



From the Geometrical Equations follows : 

dx . dO 



-~~ = a cos 6 -jr, 
dt dt 



d 2 x 



148 MECHANICS 

Combining these with (5) and reducing we obtain : 



This differential equation can be integrated by the device of 
multiplying through by 2d0/dt and then integrating each side 
with respect to t : 

30 dO 

- 



dt 
Since 



d 

it follows that 



fdO\ 2 30 . 

(dt) =-2H s 



The constant of integration, C, is determined by the initial 
conditions. If the ladder is released from rest, making an angle a 
with the horizontal, then dB/dt = and 6 = a initially, and so 

= - jj sin a + C. 

Zd 

Hence, finally, 

*> '-(-..-*.) 

To find where the ladder will leave the wall. This question is 
answered by computing R and setting it = : 



E d2 x - />d 2 */de\ 2 
R = M --trr = Ma smO-jrz Ma cos 6 [ -77 ) , 
at 1 at 2 \at/ 

(8) R = f Mg cos 6 (3 sin 6 - 2 sin a). 

Hence R = when 

3 sin 6 2 sin a = 0. 

Let ft be the root of this equation : 

ft = sin- 1 (f sin a). 
Observe that cos 8 cannot vanish when g 6 < 



DYNAMICS OF A RIGID BODY 149 

The intuitional evidence is here complete : the ladder leaves 
the wall and slides along with the lower end in contact with the 
floor. But suppose a person is unwilling to trust his intuition 
and says: "Ah, you have not proven your point in merely 
showing that R = for a certain value of 0. The ladder might 
still remain in contact with the wall, R increasing as the ladder 
continues to slide." The logic of this objection is valid. The 
objection can be met as follows. 

Think of the upper end of the ladder as provided with a ring 
that slides on a smooth vertical rod. Then the ladder will not 
leave the wall. How about R in this case? Formula (8) now 
holds clear down to the floor ; but R < when 6 < sin" 1 (| sin a), 
and so the vertical rod has to pull on the ladder instead of push- 
ing. This proves that our intuition was correct. 

The Time. From Equation (7) it appears that 



(9) 




Vsin a sin 6 

This integral cannot be evaluated in terms of the elementary 
functions. On making the substitution 

x = sin 6, 

the integral goes over into an Elliptic Integral of the First Kind, 
and can be treated by well-known methods; cf. the Author's 
Advanced CakuluSj Chapter IX. 

iii) COIN ON SMOOTH TABLE. A coin is released from rest 
with one point of the rim touching a smooth horizontal table. 
To determine the motion. 

The forces acting are: Gravity, Mg, down, and the reaction, 
R, of the table upward. Thus the centre of gravity of the coin 
descends in a right line. Let its height above the table be de- 
noted by y. Then the further Dynamical Equations become : 



(10) 



=-aRcosO. 
at* 




The Geometrical Equation is : 
(11) y osinfl. 



150 MECHANICS 

On eliminating R and y we find : 

(12) (fc 2 + a 2 cos 2 0) ^ - a 2 sin cos (9 (~f) 2 = - ag cos 0. 

(Zf \ttf / 

This differential equation comes under a general class, namely, 
those in which one of the variables fails to appear explicitly. 
The general plan of solution in such cases is to introduce a new 
variable, 



And this can be done here. But in the present case there is a 
short cut, due to the special form of the differential equation. 
It is observed that, on multiplying the equation through by 
2dQ/dt y the left-hand side becomes the derivative of a certain 
function with respect to t y so that the equation takes on the form : 

(13) 

On integrating each side of this equation with respect to t, w 
find: 



(F + o 2 cos 2 0) =-2ag sin 9 + C. 

\Gfv / 

To determine C make use of the initial conditions, dO/dt = 
and = a. Thus 

(14) (A; 2 + a 2 cos 2 ^{^) = 2a0 (sin a - sin 0). 

The angular velocity, w, of the coin when it falls flat on the 
table is given by the equation : 



_ 2ag sin a 
Wl ~ 



But here is an assumption, namely, that the point of the coin 
initially in contact with the table remains in contact till = 0. 
This is plausible enough physically; but in this gunws, is there 
not an appreciable admixture of unimaginativeness and the 
question which the moron so frequently asks: "Why shouldn't 
it?" The angular velocity dd/dt of the coin is steadily increas- 
ing, as we see both intuitionally and from (14). May it not 
increase to such an extent that the lowest point in the coin may 



DYNAMICS OF A RIGID BODY 151 

kick up and leave the table before the centre comes clear down? 
The moron certainly cannot answer this objection by physical 
intuition. 

It is here that mathematics sits as judge over the situation. 
Replace the actual problem by one equivalent during the early 
stage of the motion, and see whether this stage lasts through to 
the end. Let the lowest point of the coin be provided with a 
ring that slides on a smooth horizontal rod. Then the coin will 
fall as we guessed. Compute now the reaction, R. The test 
is: Does R remain positive throughout the motion? We leave 
it to the student to find out. 

EXERCISES ON CHAPTER IV 

1. A homogeneous solid cylinder is placed on a rough inclined 
plane and released from rest. Will it slip as it rolls, or will it 
roll without slipping? 

Ans. It will slip if the angle of inclination of the plane 
is greater than tan" 1 (|M)- 

2. The same problem for a homogeneous spherical shell 
(material surface). 

3. A billiard ball is set spinning about a horizontal axis and 
is released, just touching the cloth of the billiard table. How 
far will it go before pure rolling sets in ? 

4. A circular disc has a string wound round its circumference. 
The free end of tho string is fastened to a peg, A, and the disc is 
released from rest in a vertical plane with its centre below the 
level of A, and the string taut and vertical. Show that the 
centre of the disc will descend in a vertical right line with two- 
thirds the acceleration of gravity. 

6. The disc of the preceding problem is laid flat on a smooth 
horizontal table ; the string is carried over a smooth pulley at the 
edge of the table, and a weight equal to the weight of the disc 
is attached to the end of the string. The system is released from 
rest, the string being taut and the weight hanging straight down. 
Show that the acceleration of the weight is three-fourths that 
of gravity. 

6. Find the tension of the string in the last question. 

7. Solve the problem of Question 3 with the modification 
that the table is inclined at an angle a to the horizon. 



152 MECHANICS 

Discuss in full the case that the rotation of the ball is in such 
a sense that the ball moves down the plane faster than it would 
if it had not been rotating. 

8. Study the problem of the last question when the rotation 
is in the opposite sense. 

9. A billiard ball is placed on a billiard table inclined to the 
horizontal at an angle a, and is struck full by the cue, so that 
it starts off straight down the plane without any initial rotation. 
Study the motion. 

10. The same problem when the ball is so struck that it starts 
straight up the plane. 

11. If a man were placed on a perfectly smooth table, how 
could he turn round ? 

. 12. A plank can rotate about one end, on a smooth horizontal 
table. A man, starting from the other end, walks toward the 
pivot. Determine the motion. 

13. A smooth tube, the weight of which may be neglected, 
can turn freely about one end. A rod is placed in the tube and 
the system is released from rest with the rod horizontal. Deter- 
mine the motion. 

14. A spindle consists of two equal discs connected rigidly 
with an axle, which is a solid cylinder. The spindle is placed 
on a rough horizontal table, and a string is wound round the axle 
and carried over a smooth pulley above the edge of the table. 
A weight is attached to the lower end of the string and the system 
is released from rest. Determine the motion. 

Consider first the case in which the string leaves the axle from 
the top ; then, the case that the string leaves the axle from the 
bottom. In each case, the segment of the string between the 
axle and the pulley shall be horizontal and at right angles to the 
axis, and the part below the pulley, vertical. 

15. The centre of gravity of a four-wheeled freight car is 
5 ft. above the track and midway between the axles, which are 
8 ft. apart. The coefficient of friction between the wheels (when 
they are locked) and the track is ^-. If the car is running at the 
rate of 30 m. an h., in how short a distance can it be stopped by 
applying the brakes to the rear wheels only? How far, if the 
brakes are applied to the fronfr wheels only? 



DYNAMICS OF A RIGID BODY 153 

16. A uniform rod is suspended in a horizontal position by 
two vertical strings attached to its ends. One string is cut. 
Find the initial tension in the other one. 

17. A hoop is hung up on a peg and released. Find whether 
it will slip. 

18. A uniform circular disc, of radius 1 ft. and weight 10 Ibs., 
can rotate freely about its centre, its plane being vertical. There 
is a particle weighing 1 Ib. fixed in the rim, and a fine inextensible 
weightless string, wound round the rim of the disc, has a weight 
of P Ibs. fastened to it. The system is released from rest with 
the 1 Ib. weight at the lowest point and the other weight hanging 
freely at the same level. How great may P be, if the 1 Ib. weight 
is not to be pulled over the top? 

19. A billiard ball rolls in a punch bowl. Determine the 
motion. 

20. A solid sphere is placed on top of a rough cylinder of revolu- 
tion, axis horizontal, and slightly displaced, under the action of 
gravity. Find where it will leave the cylinder. 

21. A uniform rod is released from rest, inclined at an angle, 
with its lower end in contact with a rough horizontal plane. 
Will it slip at the start? Determine the motion. 

22. A packing box is sliding over an icy side walk. It comes 
to bare ground. Will it tip up? 



CHAPTER V 



KINEMATICS IN TWO DIMENSIONS 

1. The Rolling Wheel. When a wheel rolls over a level road 
without slipping, the nature of the motion is particularly acces- 
sible to our intuition, for the points of the wheel low down move 
slowly, the point in contact with the ground actually being at 
rest for the instant, and it is much as if the whole wheel were 
pivoted at this point and rotating about it as an axis. This is, 
in fact, precisely the case, the velocity of each point of the wheel 
at the instant being the same as if the wheel were rotating per- 
manently about that point. 

If the wheel is skidding, it is not so easy to see that a similar 
situation exists, and yet it does. No matter how the wheel is 
moving, provided it is rotating at all, there is at each instant a 
definite point (far away it may be), about which the wheel rotates 
at that instant. This point is called the instantaneous centre. 

To prove this assertion, we will begin by giving a general formu- 
lation of the problem of the motion of any plane lamina in its 
plane. It makes the problem more concrete to think of an actual 
lamina, like a disc or a triangle or a finite surface, S. But we 
are really dealing with the motion of the whole plane, thought 
of as rigid. 

The motion may be described mathematically as follows. 
Draw a pair of Cartesian axes in the moving plane; i.e. think 




X 

FIG. 90 



of this plane as a sheet of paper, and draw the (, ?/)-axes in red 
ink on the paper. Assume further a system of axes fixed in 

154 



KINEMATICS IN TWO DIMENSIONS 155 

space the (x, /)-axes. Then the (, ^-coordinates of an arbi- 
trary point P of the moving plane are connected with the (x, y)- 
coordinates of the same point by the relations : 

x = XQ + cos 6 77 sin 0, 

y 2/0 + ? sin + y c s 0- 

The position of the moving plane is known when one point, 
as 0', is known and the orientation, as given by 0, is known. 
The motion may, therefore, be completely described by stating 
how XQ, 2/0) vary with the time; i.e. by saying what func- 
tions x , 2/o> are f : 

Wo shall assume at the outset that these functions are continuous 
and possess continuous derivatives of the first order. Later, it 
will bo dosirable to restrict them further by requiring that they 
have continuous derivatives of the second order. 

EXERCISE 

Express and rj in terms of x and y y i) geometrically, by reading 
the result off from the figure ; ii) analytically, by solving Equa- 
tions A) for , 77. The formulas are : 

f f = (x - x ) cos + (y - 2/0) sin 0, 
I rj = (x XQ) sin + (y y Q ) cos 0. 

2. The Instantaneous Centre. Let P be a point fixed in the 
moving plane mark it with a dot of red ink on the sheet of 
paper. Lot the coordinates of P be (x, y). Then they are deter- 
mined as functions of t by Equations A), (, rj) being the coordi- 
nates of P with reference to the moving axes. Of course, and 
TJ are constants with respect to the time, for the red ink dot does 
not move in tho paper it moves in space. 

The vector velocity, v, of P in space can be determined by 
moans of its components along the axes of x and y y which are fixed 
in space, Chapter III, 15 : 

-^ -, -^- 



156 



MECHANICS 



These derivatives can be computed in terms of the known func- 
tions (1), namely, x , y Q , 0, and of their derivatives, by means 
of Equations A). Thus 



(2) 



dx ___ dx Q , 
dy _ dy* , f 

dt dt 



The parentheses that here enter are seen from Equations A) 
to have the values : 



Hence 



-(y- 

dx _ 
dt ~ 



X - XQ. 



~dt 



dy __ dy, , _ 
dt~~dt +(X 



dB 



These equations express the components of the vector velocity 
v of the point P along the axes fixed in space, in terms of the 
coordinates (x, y) of P and the known functions (1). 

New Notation. Since derivatives with respect to the time 
occur frequently in the work which follows, the Newtonian nota- 
tion with the dot is expedient : 



(4) 



. _dx 
X ~ ' 



x = 



dt*' 



etc. 



Thus the formula for the components of the velocity assumes tho 
final form : 



B) 



* = z - (y - 2/0) 0> 
y = 2/0 + (* - #o) * 



The Instantaneous Centre. We now inquire what point or 

points (if any) of the body are at rest at a given instant. A 

point is "at rest" if its velocity is 0. Hence the condition is, 
that x = and y = 0, or : 



(5) 



= x - (y - j/ ) 6, 
= y + (* - z n ) 6. 



KINEMATICS IN TWO DIMENSIONS 157 

These equations yield a unique solution for the unknown x 
and y when, and only when, 6 ^ : 



C) 



+ Xn 
- - - - A 



THEOREM. At any instant at which d6/dt = 6 is not 0, there is 
one and only one point of the body at rest. 

This point is called the instantaneous centre, and its coordinates^ 
( x u !/i)i are given by Equations C). 

If 6 = 0, no point of the body is at rest, or else all points are ; 
there is never a single point at rest, to the exclusion of all 
others. 

When 6 = 0, X Q and y Q not both vanishing, all points of the 
body are moving in the same direction with the same speed, 
and we have a motion of translation. 

EXERCISES 

1. Show that the coordinates (j, 77 j) of the instantaneous 
centre, referred to the moving axes, arc given by the equations : 

^o si n 6 ?y n cos & 

" 



a 

x Q cos + 2/0 sin 6 
1/1 = ^ 



2. A circle rolls on a line without slipping. Show that the 
point of contact is at rest. 

3. A billiard ball is struck full by the cue. Find the instan- 
taneous centre during the subsequent motion. 

3. Rotation about the Instantaneous Centre. The very 
name " instantaneous centre 7 ' implies that the motion of the body 
is one of rotation about that point. Let us make this state- 
ment precise. 

Suppose the body is rotating about the origin, 0, with angular 
velocity 6 = o>. What will be the vector velocity of an arbitrary 
point P:(x, y)? The answer is given by Equations B), where 
0* is taken at O, and thus x = y Q = = y Q = 0. Hence 



158 MECHANICS 

(1) f *"""* 

I y = xu. 

The result checks, for these are the components of a vector at 
right angles with the radius vector r drawn from to P and hav- 
ing the sense of the increasing angle 6, its length being 

Vx 2 + y 2 ft = ru, < 6. 

If 6 < 0, its sense is reversed. 

It is the form of Equations (1) that is important. We say 
that any motion of the points of the (x, 2/)-plane such that, at 
a given instant, the velocity of each point is given by (1), is one 
of rotation of the plane as a rigid body about 0. The velocities 
of the points in the actual motion before and after the instant in 
question may be different from those of the rigid body that is 
rotating permanently about 0. But for a short space of time 
before and after the instant, the discrepancy will be small because 
of the continuity of the motion, and at the one instant, the veloci- 
ties will all tally exactly. 

If the point about which the body is permanently rotating 
had been the point (a, 6) instead of the origin, Equations (1) 
would have been the following : 



(2) 



f *=-&-&)*, 
1 y = (x - a)6. 



We are now ready to state and prove the following theorem. 

THEOREM. The motion of the actual body at an arbitrary instant 
t, at which 6 ?* 0, is one of rotation about the instantaneous centre. 

To prove the theorem we have to show that, at the instant 2, 



where (x lt y^ are given by Equations C), 2, and (#, y} are given 
by Equations B) of the same paragraph. To do this, eliminate 
X Q and 2/ between Equations B) and C). This can be done most 
conveniently by writing Equations C) in the form (5) of 2 : 

= * - (Vi - 2/oH 
= 2/0 + (x l - x )6, 



KINEMATICS IN TWO DIMENSIONS 159 

and then, in this form, subtracting them respectively from Equa- 
tions B). The result is Equations (3) of this paragraph, and the 
theorem is proved. 

Translation and Rotation. From the foregoing result a new 
theorem about the motion of the plane can be derived at once. 
Let A be an arbitrary point, and let its vector velocity be denoted 
by V. Impress on each point of the plane, as it moves under 
the given law, a vector velocity equal and opposite to V. Then 
A is reduced to rest, and the new motion is one of rotation about 
A with the same angular velocity as before. We thus have the 

THEOREM. The field of vector velocities is the vector sum of the 
fields consisting i) of the translation field due to the vector velocity 
of an arbitrary point, A ; and ii) of the rotational field with A as 
centre. 

In other words, the given motion consists of rotation about an 
arbitrary point, A, plus the translation of A. 

The theorem also follows immediately from Equations B), if 
we take the point 0' at A. 

4. The Centrodes. We are familiar with the motion of a 
circular disc when it rolls without slipping on a right line or a 
curve a wheel rolling on the ground. Con- 
sider, more generally, the motion of a lamina 
when an arbitrary curve drawn in it rolls 
without slipping on an arbitrary curve fixed 
in space. Wo may think of a brass cylinder, 
or cam, as cut with its face corresponding to 
the first curve, and attached to the body; 
a second such cam, with its face corresponding to the second 
curve, being fixed in space. And now the first cam is allowed 
to roll without slipping on the second cam. 

Thus a great variety of motions of the lamina can be realized, 
and now the remarkable fact is that all motions can be generated 
in this way, with the single exception of the translations, 
provided that the functions (1) of 1 have continuous deriva- 
tives of the second order, and the space centrode is traced out 
by the instantaneous centre with non-vanishing velocity. 

A necessary condition for the truth of this statement is evident 
from intuition, namely : the point of contact of the two cams 




160 MECHANICS 

must be the instantaneous centre of the actual motion. This fact 
suggests the proof the faces of the cams, i.e. the curves, must 
be the loci of the instantaneous centres in the body and in space. 
Definition. The locus of the instantaneous centre in the body 
is called the body centrode, and the locus of the instantaneous 
centre in space is called the space centrode. 

THEOREM. Any motion of a rigid lamina which is not transla- 
tion can be generated by the rolling of the body centrode (without 
slipping) on the space centrodc, provided the space centrode is traced 
out by the instantaneous centre with non-vanishing velocity; the 
functions (1) of 1 having continuous derivatives of the second order. 

Before wo can prove the theorem, we must make clear to our- 
selves how to formulate mathematically the rolling of one curve 
without slipping on a second curve. As the independent variable, 
the *timo most naturally suggests itself; but it is better at the 
outset not to choose it, but to take, rather, a variable X which 
merely corresponds to tho fact that, for an arbitrary (i.e. variable) 
value of X, the curves meet in a (variable) point P. And now 
we shall demand further : 

i) that the curves be tangent to each other at P ; 

ii) that the arc of the one curve corresponding to any two 
different values of X, namely, Xj and X 2 ; and the arc of the other 
curve corresponding to the same values of X, have the same length. 

Thus, in particular, both curves may be moving a more 
general case than the one that interests us here. 

Let the equation of the one curve, C, referred to a system of 
Cartesian axes, (x, y), be : 

(1) * = ff(A), = A(X), 

where the functions #(X), h(\) are continuous together with 
their first derivatives, and the latter do not vanish simultane- 
ously : 

(2) <<7'(X) 2 + /i'(X) 2 . 

Let the second curve, F, referred to a second system of Cartesian 
axes, (, r;), be represented by similar equations, 

(3) 

(4) 



KINEMATICS IN TWO DIMENSIONS 



161 



The coordinates of any point of the plane, referred to the one 
set of axes, are connected with the coordinates of the same point, 
referred to the other set of axes, by the equations : 

x = x + % cos 6 TI sin 0, 
y = 2/o + sin 9 + rj cos 0. 

And now we require that X Q , y Qy 6 be functions of X which have 
continuous first derivatives : 



(5) 



(6) *o=/00, 2/o=* 00, = 

where /'(X), ^'(X), ^'(X) exist and are continuous. 

Since C and F always meet in a point P, whose coordinates 
are expressed by the equations (1) and (3), it follows that Equa- 
tions (5) will hold identically in X if the values of x } y from (1), 
and those of , 77 from (3), be substituted therein. 

The vector v whose components are 

_ dx __ dy 

Vx ~ d\' Vy ~~ d\ 

is tangent to C at P and its length is 



The vector u whose components arc 



is tangent to F at P and its length is 



The requirements i) and ii) demand that these two vectors 
be identical. This condition is both necessary and sufficient. 
The analytical formulation of tho condition is as follows : 



(7) 



v x = u$ cos B Uy sin 0, 
v y = u% sin B + u^ cos B. 



We now have all the material 
out of which to construct the 
proof. From Equations (5) it 
follow? that 




FIG. 92 



162 MECHANICS 

dx 






The first line in these equations is nothing more or less than 
the first of Equations (7), and the latter equations we have set 
out to prove. Hence the second line must vanish, if the equation 
is to be true, and so, by the aid of (5), we obtain the first of Equa- 
tions (8) : 



< 8) 



The second equation is obtained in a similar manner from the 
second of the above equations. 

Equations (8) represent a new form of necessary and suffi- 
cient condition for the fulfilment of Conditions i) and ii). 

5. Continuation. Proof of the Fundamental Theorem. It 

is now easy to prove the theorem of 4. The two curves, C 
and F, are here the space centrode and the body centrode, and 
we will now take as our parameter X, the time t. Equations (1), 
4, thus represent the coordinates, x l and y lt of the instanta- 
neous centre in space, and in Equations (8), the (x, y) are the 
coordinates of this same point, (x l9 yj. The other quantities 
that enter into (8) are the functions (6) that determine the posi- 
tion of the moving body; and X = t. Thus Equations (8) go 
over into the following : 

f *o - (2/i - 2/o) * = 0, 
1 2/o + (x l - z ) 6 = 0. 

But these are precisely Equations (5) of 2, which determine the 
instantaneous centre. Equations (8) are thus shown to be true. 



KINEMATICS IN TWO DIMENSIONS 



163 



Discussion of the Result. From Equations (8) 4, it appears 
that a necessary condition for the truth of the theorem is, that 
the coordinates of a point P of C satisfy the equations : 



(10) 



X = X n - 



dy /d0 
dX / dX' 



, dx a I dB 
y = 2/o + -3r / 3T- 



But these conditions are not sufficient, since the functions x and 
y thus defined will not in general admit derivatives. 

To meet this latter requirement we demand, therefore, that 
the functions (6) possess, furthermore, continuous second deriv- 
atives. But this is not enough, even if the case that x and y 
reduce to constants is excluded (rotation about a fixed point). 
It is, however, sufficient when we add the hypothesis of (2), 
4, and so demand that 



dy / de \ 
~dx/dx/' 



d 



de 



be not both (dO/d\ being, of course, 5^0). In other words, 
the equations 



(12) 

t 



d0 d 2 x _ d^cteo _, ^!^o = 
dX dX 2 dX 2 dX "*" dX 2 dX U| 

dX'dX 2 " "" dX*"d\ "~ dX 2 dX = 



shall never hold simultaneously. This excluded case includes 
the case in which an ordinary cusp occurs; but it also includes 
more complicated singularities. 

If, in particular, the functions (6) are analytic in the neighbor- 
hood of a point, X = X , and if the case of permanent rotation 
about a fixed point be excluded, the curve C will at most have 
a cusp and otherwise be smooth in the neighborhood of the point ; 
and the same will be true of P. 

Acceleration of the Point of Contact. Let the point (X Q , y ), 
at a given instant, t, be taken at the point of contact of C and T. 
Then it follows from (10) or, more simply, from (8) since 
x = x Q and y = y Q> that 



dX 



164 MECHANICS 

Let the origin, furthermore, be taken at this point (x , y ), and 
let C be tangent to the x-axis here. Now, the derivatives of x 
and y in (10) cannot both vanish. On computing them it is 
seen that they reduce respectively to 



d\ 2 ~d\' d\ 2 d\ 

The second, dy/d\, has the value 0, since C is tangent to the axis 
of x at the origin. Hence we infer that 



If X is the time, t, these derivatives become the components 
along the axes of the acceleration of the point of contact, thought 
of as a point fixed in the moving body. From (13) it appears that 
this acceleration is never 0, but is a vector orthogonal to the 
centrodes at their point of contact. The reader can verify this 
result in the case of the cycloid. 

Example. A billiard ball is projected along a smooth hori- 
zontal table with an initial spin about the horizontal diameter 
which is perpendicular to the line of motion of the centre. Deter- 
mine the two centrodes. 

Take the path described by the centre of the ball as the axis of x, 
and the centre of the ball as (x , y ). Then 

Equations (10) give : 
FIG. 93 x = X Q , y =--. 

Hence the space centrode is a horizontal straight line at a distance 
c/co below the centre of the ball, and the instantaneous centre 
is always beneath the centre of the ball. This means that the 
ball rolls without slipping on a right line distant c/w below the 
centre. Hence the body centrode is a circle of radius c/co about 
the centre of the ball. 

EXERCISE 

A billiard ball is struck full by the cue. Determine the 
space centrode and the body centrode during the stage of slipping ; 
cf. Chapter IV, 14. 




KINEMATICS IN TWO DIMENSIONS 



165 



The coordinates being chosen as in the Example, the equations 
of the space centrode are : 

SC ~~ *C rt ~~ Cv """" 



_ 2a _ 
V ~ 5 



2acl 
5/ t' 



where a denotes the radius of the ball, and c the initial velocity 
of its centre. The time that elapses during the stage of slipping 
is 2c/7/A<7 seconds. The space centrode meets the billiard table at 
the angle 



The equations of the body centrode, referred to suitable polar 

coordinates, are : 

2ac 1 2a 



P =- 



t 



5 ' 



6. The Dancing Tea Cup. When an empty tea cup is set 
down on a saucer, the cup sometimes will dance for a long time 
before coming to rest. Two features of this phenomenon attract 
attention; first, that the energy, obviously slight, is not earlier 
dissipated by damping, and secondly, that we can hear a noise 
in which so little energy is involved. The second point can be 
disposed of easily because of the physical fact that the energy 
of sound waves is surprisingly small. 

To examine the first critically we need more light on the nature 
of the motion. The results which wo have obtained in this 
chapter furnish the clue. The following example is highly sug- 
gestive. 

Consider the motion of a lamina, in which 
the body centrode is a right line making a 
small (variable) angle with the horizontal. 
For the space centrode take a curve suggested 
by the figure. Such a curve can be defined 
suggestively as follows. Begin with the curve 



(1) 



y = sin - 




166 MECHANICS 

This curve gives satisfactorily the part of the figure not too near 
the lines y = 1, but it is tangent to these lines, whereas it 
should have cusps on them. 

The desired modification is simple. For example, to convert 
the curve 

y=f( X )= X * 

from one which is tangent to the axis of x into one which has a 
cusp on the axis, it is enough to replace f(x) by [/(z)]* : 



Apply this idea to the curve (1). It will suffice to set 
(2) y 



as the reader can easily verify. 

Now allow the body centrodo the tangent line to descend 
according to a reasonable law. We have here a picture of what 
goes on as the tea cup dances. The line oscillates through smaller 
and smaller angles as its point of intersection with the axis of x 
descends. 

Tyndall,* in his popular lectures, showed an experiment with 
a coal shovel illustrating the same phenomenon. The all-metal 
shovel was heated near its centre of gravity and laid across two 
thin lead plates clamped in a vise, with their edges horizontal. 
As the shovel bore more heavily on one of the plates, the latter 
expanded with the heat, throwing the shovel onto the other 
plate. Then the process was reversed. Thus vibrations like 
those of the tea cup arose, and died down. 

7. The Kinetic Energy of a Rigid System. The kinetic en- 
ergy of any system of particles is defined as 

T = i 2) m ^\ v k 2 = x k 2 + yi 2 + zt 2 . 

We restrict ourselves to two dimensions, and thus 

vi? = xj? + yj?. 

Suppose, now, that the particles are rigidly connected. In 
Equations A), 1, let the point (x , y ) be taken at the centre 
of gravity, (x, y). Thus Equations (2), 2, become : 

* Tyndall, Heat Considered as a Mode of Motion, Lecture IV. 



KINEMATICS IN TWO DIMENSIONS 167 

k = x (& sin + *;* cos 0) 0, 
Vk = + (& cos - 77* sin 0) 0. 

On squaring and adding, multiplying by m k , and then adding 
with respect to k, we find : 



For, each of the remaining terms involves as a factor one of the 
quantities 

2) 



and each of these is 0, since the centre of gravity is at the origin 
of the (, 7y)-axes. Hence it follows that 

(1) T = |MF 2 + i/fl 2 , 

where V denotes the velocity of the centre of gravity and I is the 
moment of inertia about the centre of gravity, 12 being the angular 
velocity. 

Second Proof. The result may also be obtained by means of 
the instantaneous centre, 0. For the motion, so far as the 
velocities that enter into the definition of T are concerned, is 
one of rotation about 0. Hence 

(2) T = i/'ft 2 , 

where /' denotes the moment of inertia about 0. Now, 

/' = I + Mh\ 
where h is the distance from to the centre of gravity, and 

(3) V = Aft. 

On substituting this value of /' in (2) and then making u$e of (3), 
T takes on the form (1), and this completes the proof. 

Generalization. The most general rigid bodies with which we 
are concerned are made up of particles and material distribu- 
tions spread out continuously along curves, over surfaces, and 
throughout regions of space. When such a body rotates about 
an. axis, the kinetic energy is defined by Equation (1). We 
can state the result in the form : 

The kinetic energy of any rigid material system which is rotating 
about an axis, is given by the formula: 

T 



168 MECHANICS 

Remark. The formula holds even for the most general case of 
motion of any rigid distribution of matter in space. For, such 
motion is helical, i.e. due to the composition of two vector fields 
of velocity, i) a field corresponding to rotation about an axis; 
and ii) a field of translation along that axis ; cf . 12 below. 

EXERCISES 

1. A ball rolls down a rough plane without slipping. Deter- 
mine the kinetic energy in terms of the velocity of its centre. 

2. A ladder slides down a wall, the lower end sliding on the 
floor. Find the kinetic energy in terms of the angular velocity. 

3. A uniform lamina in the form of an ellipse is rotating in 
its plane about a focus. Compute the kinetic energy. 

4. A homogeneous cube is rotating about one edge. Determine 
the kinetic energy. 

8. Motion of Space with One Point Fixed. Consider any 
motion of rigid space, one point, 0, being fixed. We shall show 
that there is an instantaneous axis, i.e. a line through 0, the 
velocity of each point of which is 0; and that the velocities of 
all the points of the moving space, considered at an arbitrary 
instant, form a vector field which coincides with the vector field 
arising from the permanent rotation of space about this axis. 

We give first a geometrical proof which appeals strongly to 
the intuition. The refinements which a critical examination 
of the details calls for are best given through a new proof by 
vector methods. 

Let Q be a point of the fixed space, distinct from O. If its 
velocity is 0, then the velocity of every point of the indefinite 
right line through and Q is 0, since a variable right line is evi- 
dently at rest if two of its points are at rest. 

If, on the other hand, Q is moving, pass a sphere, with centre 
at 0, through Q and consider the field of vector velocities cor- 
responding to the points of this sphere. The vectors are evidently 
all tangent to the sphere, and they vary continuously, together 
with their first derivatives, for we are not concerned with dis- 
continuous motions. 

Pass a great circle, (7, through Q perpendicular to the vector 
velocity of Q. Let P be a point of C near Q. Then the vector 



KINEMATICS IN TWO DIMENSIONS 169 

velocity of P will also be at right angles to the plane of C and on 
the same side of C as the vector at Q. For, since the vector 
velocity of Q is at right angles to the chord QP, the vector velocity 
of P must lie in the plane through P perpendicular to QP. But 
it also lies in the tangent plane to the sphere at P. And now I 
say, there, must be a point A of C (and hence two points) whose 
velocity is 0. For, otherwise, all the vectors that represent the 
velocities of the points of C would be directed toward the same 
side of C. In particular, then, the point Q' diametrically opposite 
Q would have such a vector velocity. But that would mean 
that the mid-point of the diameter Q'Q, i.e. the centre of the 
sphere, is not at rest. From this contradiction follows the truth 
of the assertion that there is a point A of C which is at rest. Hence 
the whole indefinite line through and A is at rest, and the exist- 
ence of an instantaneous axis, 7, is established. 

Rotation about the Instantaneous Axis. It remains to prove 
that the vector field of the actual velocities coincides with the 
field of the vector velocities due to a rotation about I. Con- 
sider an arbitrary point, P, not on /. Then P cannot be at 
rest, unless all space is at rest. For, if three points, not in a line, 
of moving space are at rest, all points must be at rest. Pass 
a plane, M, through P and the axis. Then the vector velocity 
of P must be perpendicular to M. For let Q be any point of /. 
Since Q is at rest, the vector velocity of P must lie in a plane 
through P perpendicular to QP. 

Consider next the circle, C, through P with / as its axis. The 
vector velocity of P is tangent to C. For it is perpendicular to 
any line joining P with a point of /. Moreover, the vector 
velocities of all points of C are of the same length. For other- 
wise two points of C would be approaching each other, or reced- 
ing from each other.* 

Lastly, the magnitude of the vector velocity of P is propor- 
tional to its distance from /. Let M be the plane determined 
by 7 and P. Consider two points, P 1 and P 2 , in M but not on 
7, distant A, and h 2 respectively from 7. Let uh l be the magni- 
tude of the vector velocity of P t . Then coA 2 is the magnitude of 
the vector velocity of P 2 . For otherwise P 2 would issue from 
the rigid plane M.f This completes the proof. 

* Exercise 4 below. t Exerciso 5 



170 



MECHANICS 



EXERCISES 

1. Give a rigorous analytic proof that if two points of a moving 
straight line are at rest, every point of the line is at rest. 

2. A point Q is moving in any manner, and a second point, P, 
is so moving that, at a given instant, it is neither approaching Q 
nor receding from Q. Give a rigorous analytic proof that the 
vector velocity of P is orthogonal to the line QP, if the vector 
velocity of Q is orthogonal to that line. 

3. If three points of space are at rest, and if these points do 
not lie on a line, all space is at rest. Prove rigorously analyt- 
ically. 

4. Prove analytically the statement of the text which refers 
to this Exercise. 

5. The same for this statement. 

9. Vector Angular Velocity. Let space rotate as a rigid body 
about a fixed axis, L, with angular velocity o>. Let P be an 
arbitrary point fixed in the moving space. 
Then the velocity of P will be represented by 
a vector v perpendicular to the plane deter- 
mined by P and the line L, and of length 
hw, where h is the distance of P from L. 

Let be any point of L. Lay off from 
along L a vector of length w and denote this 
vector by (co). Let r be the vector drawn from O to P. Then 
the vector velocity v of P is represented by the vector product 
of (w) and r : 




FIG. 95 



(1) 



Xr; 



cf. Appendix A. 

Let a system of Cartesian axes (or, y, z) be assumed with as 
origin, and let i, j, k be unit vectors along these axes. Write 



(2) 
Then 

(3) 



co 2 k. 



i J k 



x y z 



KINEMATICS IN TWO DIMENSIONS 171 

The components of v along the axes are thus seen to be : 



v x = 

Vy = XUg ZO) 

Vg = 



(4) 



Composition of Angular Velocities. Consider two rotations about 
axes which pass through 0. Let them be represented by the 
vectors (o>) and (a/)- An arbitrary point P of space has a vector 
velocity v given by (1) : 

v = () X r, 

due to the first rotation, and a vector velocity v' : 

V = (') X r, 

due to the second rotation. 

Let these vectors, v and v', be added. Then a third vector 
field results one in which to the point P is assigned the vector 
v + v'. It is not obvious that this third vector field can be 
realized by a motion of rigid space far less, then, that it is 
precisely the field of velocities due to the angular velocity repre- 
sented by the vector 

(5) (0) = () + (0- 

That this is in fact true that is the Law of the Composition of 
Angular Velocities. 
The proof is immediate. We have : 

(6) v + V = () X r + (') x r. 
Now, the vector, or outer, product is distributive : 

(7) {() + (')} X r = () X r + (') X r. 

Hence 

(8) v + v' = {() + (a/)} X r = (12) X r, 

and we are through. The result can be formulated as the fol- 
lowing theorem. 

THEOREM. Angular velocities can be compounded by the Law 
of Vector Addition. 

EXERCISE 

Prove the law of composition for angular velocities by means 
of Equations (4). 



172 



MECHANICS 



10. Moving Axes. Proof of the Theorem of 8. Let space 
be moving as a rigid body with one point, 0, fixed. Let i, j, k 
be three mutually orthogonal unit vectors drawn from and fixed 
in space, and let a, 0, 7 be a second set of such vectors fixed in 
the body. The scheme of their direction cosines shall be the 
following : 

a j8 7 rj f 



(1) 
Thus 



'l '2 



a = 



with similar expressions for /3, 7, where the direction cosines 
are any functions of the time, t, continuous with their first (and 
for later purposes their second or even third) derivatives, and 
satisfying the familiar identities ; cf. Appendix A. Observe that 



(2) 



187 = 



aa = 0, etc. 
07 + 7/3 = 0, etc. 
We are now in a position to prove analytically the existence of 
an instantaneous axis. Let P be an arbitrary point fixed in the 
body, and let r be the vector drawn from the fixed point to P. 
Then 

(3) r = f a + vp + f 7. 

Since P is fixed in the body, , 77, f are constant with respect 
to the time, and so 

(4) t = $a + 40 + fy. 

A necessary and sufficient condition that P be at rest is, that 
the projections of f on three non-complanar axes all vanish. 
Hence, in particular, the condition that P be at rest can be ex- 
pressed in the form : 

(5) at = 0, fit = 0, 7* = 0. 

Applying this condition to the vector (4), we find the three 
ordinary equations : 



KINEMATICS IN TWO DIMENSIONS 173 



+ f ay = 
(6) tfa+ f 07 = 

=0 



Let 

(7) a = yp, b = ay, c = pa. 
From (2) it follows that 

a = pj y b = 7, c = aft. 

Equations (6) arc now seen to admit the particular solution: 
= a, 77 = b, f = c. 

These cannot all be unless the body is at rest, since the vanishing 
of the above scalar products would mean that 

pa = 0, ya = ; 

and of course aa = 0. Thus the vector a would be at rest, and 
likewise, each of the other vectors, P and 7. 

The general solution of the equations (6) is given by the equa- 
tions : 

(8) = Xa, ij = X6, f = Xc, - oo < X < oo . 

These points, and these only, are at rest. They form the instan- 
taneous axis, and it remains to show that the* latter deserves 
its name. 
Instantaneous Axis. Let a vector (co) be defined as follows: 

(9) o> = 7/3, a, = ay, co$ = fta ; 

(10) (CO) = C00! + ^0 + W^7. 

Then (co) is collinear with the instantaneous axis, whose equa- 
tions (8) can now be written in the form : 

(11) 1 = JL = L. 

CO^ COr, CO^ 

We have seen that the vector velocity v of an arbitrary point 
fixed in the body is given by (4). The components of v along 
the (, 77, f )-axes can be written in the form : 

V{ = at = %aa + yap + f ay 



= yt = %ya + rjyp + yy 



174 MECHANICS 

Hence 

ff = f 

From (12) it follows that 



(13) V = COf W, CO^ = (CO) X T, 

r 

and so we see that the actual vector velocity v of P is the same 
as the vector velocity which P would have if rigid space were 
rotating about the instantaneous axis with angular velocity co. 

Thus the actual field of vector velocities of the points P coin- 
cides with the field of vector velocities due to rotation about the 
instantaneous axis represented by the vector angular velocity 
(co), and the proof is complete. 

11. Space Centrode and Body Centrode. The locus of the 
instantaneous axis in fixed space is called the space centrode, and 
its locus in the moving space, the body centrode. The actual 
motion consists of the rolling of the one cone (the body centrode) 
without slipping on the other cone (the space centrode). 

To prove this statement consider the path traced out by a 
specified point in the instantaneous axis. Take, for instance, 
the terminal point of the vector (co), the initial point being at 0. 
The locus of this point is a certain curve C on the space centrode : 

(co) = co x i + coj + cosk, 
and a certain curve T of the body centrode : 

It is sufficient to show that these curves are tangent and that 
corresponding arcs are equal. This will surely be the case if 
d(u>)/dt for C is equal to d(co)/cft for F. Now, the first vector 
has the value 

The value of the second vector is : 

+ a*,/? + co$ 



KINEMATICS IN TWO DIMENSIONS 175 

The last line vanishes because it represents the velocity of 
the point (o>) fixed in the body, this point lying on the instan- 
taneous axis. The first line is the vector (co). This completes 
the proof. 

EXERCISE 

Treat the motion of the plane by analogous vector methods. 
Let _ 



be the vector drawn from the fixed to the moving origin, and 
let p, a- be unit vectors drawn along the positive axes of and rj. 
Let r be the vector from the fixed origin to an arbitrary point P. 

Then 

r = f + p + r?<7. 

The vector velocity in space of a point P fixed in the plane is 
given by the vector equation : 

* = f + f P + ^- 

The instantaneous centre is given by setting t = 0. 
On the other hand, 

p = e", a = C + D'. 



The complete treatment can now be worked out without diffi- 
culty. 

12. Motion of Space. General Case. Let rigid space be 
moving in any manner, subject to the ordinary assumptions 
about continuity. Reduce a point A to rest by impressing on 
all space a motion of translation whose vector is equal and oppo- 
site to the vector velocity of A. The vector field of the velocities 
in the original motion is compounded by the parallelogram 
law of vector addition out of the two vector fields i) of translation 
and if) of rotation about the instantaneous axis, 7. 

Let the vector that represents the translation be resolved into 
two vectors, one, T, collinear with 7, the 
other, A, at right angles to 7. The velocity ~H 
of any point, P, distant h from the axis, is, 
in the case of pure rotation, hu ; its direc- 
tion is at right angles to the plane through P and the axis, and its 
sense is a definite one of the two possible senses. Hence it is seen 



176 MECHANICS 

that it is possible to find a point, B, whose vector velocity due to 
the rotation is equal and opposite to the vector velocity A. (Draw 
a line from a point of the axis, perpendicular to / and A, and 
measure off on it, in the proper direction, a distance h = A/u.) 
All points in the line L through B parallel to / will also be at 
rest. It thus appears that the original motion is one of rotation 
about L compounded by the law of vector addition with a motion 
of translation parallel to L tiad represented by the vector T. 

This vector field is, in general, the same as that of the vector 
velocities of the points of a nut which moves along a fixed machine 
screw (or of the points of a machine screw which moves through 
a fixed nut). The two exceptional cases are those of rotation, 
corresponding to a pitch of the threads, and translation, the 
limiting case, as the pitch becomes infinite. 

13. The Ruled Surfaces. We have seen in 12 that the 
vector field of velocities, in the general case of the motion of rigid 
space, is the sum of two vector fields one, rotation about an 
axis, L ; the other, translation parallel to L. The locus of L in 
space is a ruled surface S, the space centrode, and the locus of L 
in the moving space is also a ruled surface, S, the body centrode. 
From analogy with the rolling cones we should anticipate Jhe 
theorem governing the present case. 

THEOREM. The surface is tangent to S along L, and it rolls 
and slides on S. 

An intuitional proof can be given as follows. First of all, it 
is clear from the very definition of L that S slides on S along L. 
So it is necessary to prove only the tangency of the two surfaces. 
Let L be the line L at time t = , and let P be a point of L . 
Pass a plane through P perpendicular to L , cutting S in the 
curve Cj and let P be the point in which L at time t = t Q + At 
cuts C. Let Q be the point fixed in S, which will coincide with 
P at time t Q + A. The vector velocity of Q at the instant t 
t has a component, c, parallel to L and a component hu at right 
angles to the plane through L and Q. Obviously h is infinitesimal 
with AJ. In time M the point Q will, then, have been displaced, 
save as to an infinitesimal of higher order, parallel to L by a 
distance cAt. But it will have reached P. 

The proof is now clear. The plane through L and Q makes 
an infinitesimal angle with the tangent plane to S at P Q because 



KINEMATICS IN TWO DIMENSIONS 177 

it contains a point Q of S infinitely near to P , but not on L . 
The plane through L and P makes an infinitesimal angle with 
the tangent plane to S at P Q because it contains a point P of S 
infinitely near to P , but not on Z/ . And these two planes make 
an infinitesimal angle with each other, because when Q is dis- 
placed parallel to L by a distance cA, its distance from P is an 
infinitesimal of higher order than the distance of P from P . 

Instead of developing the details needed to make the intuitive 
proof rigorous, we will treat the whole question by vector methods. 
First, however, a digression on relative velocities. 

14. Relative Velocities. Let a point P move in any manner 
in space, and let its motion be referred to a system of moving 
axes. 

Consider, first, the case that the moving axes have a fixed 
origin, 0. Let a system of axes (x, y, z), fixed in space, with 
origin at be chosen ; let the moving axes be denoted by (, 77, f), 
and referred to the fixed axes by the scheme of direction cosines 
of 10. Let r be the vector drawn from to P : 

0) r = f + 4/9 + [ 7. 

Then 



or 

(3) v = v r + v, 

where the terms on the right have the following meanings. The 

vector, 

,.. d , drj _ , df 

< 4 > ^-dr + s'- 1 -*" 

represents the velocity of P relative to the moving axes; i.e. 
what its absolute velocity would be if the (, t;, f)-axes were fixed 
and P moved relative to them just as it actually does move. 
Secondly, the vector 

(5) v e = ** + it + r 7 

represents the velocity in space of that point fixed in the body, 
which at the instant t coincides with P. To say the same thing 
in other words : Let us consider the point P at an arbitrary 
instant of time, t = t. Let Q be the point fixed in the body, 



178 



MECHANICS 



which at this one instant coincides with P. Then v e is the vector 
velocity of Q. It is the vitesse d'entrainement, the velocity with 
which the point Q is being transported by the body at the instant t. 
The analytic expression for v e we know all about. In vector 
form it is : 

(6) v e = () X r 

or 



(7) 



Its components along the axes, if we write v' = v ej are : 



(8) 



Thus we have as the final solution of our problem this: The 
components of the vector velocity of P along the axes of % , ry, f are : 



(9) 



= + 



General Case. Let the axes of (x, y, z) be fixed in space. 
Let (, TJ, f) be the moving axes, whose origin, 0', has the coor- 
dinates (X Q , i/o, 2 ). Then 

(10) r = r + r'. 
Hence 

(11) v = v + v'. 
Here, 




FIG. 97 



(12) 



dx Q . 



and v' is given by (9). The v' of (11) is, of course, not the V 
of (8). 



KINEMATICS IN TWO DIMENSIONS 
EXERCISE 



179 



Denoting the components of v along the ( , 17, f )-axes by 
> v*y v l> show that the components of v along these axes are : 



(13) 



Here, 






dy 

'dt + ^~ 
4 + 



= 7*0. 



16. Proof of the Theorem of 12. Let a system of Cartesian 
axes fixed in space, (x, y, 2), with origin in be assumed. Let 
O' : (x , y^ ZQ) be a point fixed in the body, the motion of 0' 
being known : 

(1) *o=/(0, 2/o = v(0, *o = lKO. 
Finally, let P be any point fixed in the body. Then 

(2) r = r c + r', 

cf. 14, (10) with the specialization that here 



(3) 



dt 



Then the components of the absolute velocity of P (i.e. its velocity 
in fixed space) along the axes of ( , 77, f ) are given by the formulas 
of 14, 13 : 



(4) 



We can formulate the problem as follows : To find a point 
^(i> i/D fi) fixed in the moving space whose absolute vector 
velocity is collinear with the vector (o>), or is : 

(5) *, = (<>). 

Here, (co) is the vector angular velocity of the moving space, 
whose rotation is defined by the direction cosines of 10. 



180 



MECHANICS 



By virtue of (4) the vector equation 
three ordinary equations : 



(6) 



(5) is equivalent to the 



Since 



(7) 







- 



= 0, 



a further necessary condition is : 
(8) utat + co^f 

We can dispose at once of the case o> = ; for then the space 
in which 0' is at rest, is stationary, and so the motion of the given 
space is translation (unless it be at rest). Thus all lines parallel 
to the vector that represents the translation are axes such as 
we seek. 

If o) ^ 0, we obtain from (8) a unique determination of k. 
On substituting this value in (6), two of these equations, suitably 
chosen, determine uniquely two of the three unknowns lf rj l} f t 
as linear functions of the third, and then the remaining equation 
(6) is true because of (8). 

i = i> i7i = 61, fi = c i 

be a particular solution of (6), then an arbitrary solution, 
i 'Ju Ti> will satisfy the equations : 



(1 - fli) 



+ (fi - c iK = 
- (f i - c^cu* = 



Hence 
(9) 



and thus &, T^, ft is seen to be any point of the line through 
(a,, bi, Cj) collinear with (<*>). This line we define as L. These con- 
ditions are sufficient as well as necessary. 



KINEMATICS IN TWO DIMENSIONS 181 

The locus of L in space is the ruled surface S ; its locus in the 
body (i.e. the moving space) is the surface S. These surfaces 
have the line L in common. We wish to show that they are 
tangent along L, and that S slides over S in the direction of L. 
The last fact is clear from the definition of L. 

The point (&, rj lf f t ) is not uniquely determined by the time, 
but may be any point of L. We will, for our purposes, select it 
as follows. Let Z/ be a particular L, and let P be an arbitrary 
point of L , once chosen and then held fast. Pass a plane M 
through P orthogonal to L . Then (x lf y lt zj shall be the inter- 
section of the variable line L with M , and its locus shall be denoted 
by C. The point (f t , y ly fj shall be the point of S which coin- 
cides with (xu yi, 2i) at time t = t. Its locus in S shall be denoted 
by F. This curve can be represented in the form : 



F: ti=F(t), 77! = $(0, fi=*(0- 

Its tangent vector at an arbitrary point is 

k a + *?i* + #, 

dt + dt 1 * + dt 7 ' 

provided this vector 7* 0. 

To show that two surfaces which intersect at a point P are 
tangent it is sufficient to show i) that they have a common tangent 
vector, t ; and ii) that a tangent vector tj to the one surface and 
a tangent vector t 2 to the other surface, neither collincar with t, 
are complanar with t, all three vectors, emanating from P . 

The surfaces S and 2 satisfy i) because they are both tangent 
to L. Secondly, consider the vector ^ drawn from to the point 
of intersection of C and F at time t t. Its derivative is a vector 



tangent to C, provided it 5^ 0. 

On the other hand, consider the point (| t , 77^ J\) of F, for which 
t = t. Let the vector drawn from 0' to this point be denoted 
by r[. Then 

*i = TO + i{, 

where r is given by (1), and 



182 MECHANICS 

Hence 

^ -^tt-L*'!* j-*j,y 

dt " dt a ^'M ft ^ dt y 
4-fo + ^d + 7/^ + ^7. 

This last line is precisely the vector velocity of that point fixed 
in S, which at the instant in question, t = t, coincides with 
( x \> V\y z i)- This vector, t, let us call it, lies along L because of 
(5), unless it be 0. 

The other vector on the right of (11) is the vector (10); i.e.. 
a vector t 2 tangent to T at (, rj ly f,) or (x l9 y lt zj. Equation 
(11) thus says that 

ti = t, + 1. 

Now, the vector drjdt = t x ^ will not lie along L. Hence t. 2 
will not, either. Consequently Condition ii) is satisfied, arid the 
surfaces S and F are tangent along L. The case t = is included ; 
it does not lead to an exception. 

EXERCISE 

Let a cylinder of revolution roll and slide on a second cylinder 
which is fixed, the first cylinder always being tangent along an 
element, and there being no slipping oblique to the element. 
Choose the point (x , i/ , z ) in the axis of the moving cylinder, 
and discuss the whole problem by the method of this paragraph. 

16. Lissajou's Curves. In one dimension, or with one degree 
of freedom, the most important periodic motion is Simple Har- 
monic Motion. It can be represented analytically in the form : 

(1) x = a cos (nt + 7), 
where 

(2) T = - 

' n 

is the period, where a is the amplitude, and where 7 is determined 
by the phase. 

In two dimensions, or with two degrees of freedom, an impor- 
tant case of oscillatory motion about a fixed point is that in 
which the projections of the moving point on two fixed axes 



KINEMATICS IN TWO DIMENSIONS 183 

at right angles to each other, execute, each by itself, simple har- 
monic motion : 

I x = a cos (nt + 7) 

\u) 1 

I y = b cos (mi + e) 

It is possible to generalize at once to n dimensions : 
(4) x k = a k cos (n k t + y k ), fc = Z, , n. 

Let us study first the two-dimensional rase, beginning with 
some simple examples. We may set 7 = if, as usually hap- 
pens, the instant from which the time is measured is unimpor- 
tant. 

Example 1 : m = n. Dynamically, this case can bo realized 
approximately by the small oscillations of a spherical pendulum. 
Let 7 = 0, 

<p = nt. 
Then 

mt + e = <f> + , 

(x = a cos <p 
y = A cos <p B sin <p 

A = b cos e, B = b sin c. 

Assume that neither a nor b vanishes, since otherwise we should 
be thrown back on right line motion along one of the axes. We 
will take a > 0, b > 0. 

In general, B ^ 0. The path of the moving point is then 
an ellipse with its centre at the origin. For, 

(6) cos <p = ^, sin <p = -^ x - ^ y. 

On squaring and adding we find : 

(7) B 2 x 2 + (Ax - ay) 2 = a 2 B 2 , 

and this equation represents a central conic which does not reach 
to infinity, i.e. an ellipse. 



184 MECHANICS 

The axes can be found by the methods of analytic geometry, 
or computed directly by making the function 

COS 2 ^ __ 2AB cos <p sin ^ + B* sin 2 ^ 



We have omitted the special case : B = 0. Here, e = or 
TT, and the motion is rectilinear, along the line : 



In all cases, the path is confined within the rectangle : 
x = a, y =b, 

and continually touches all four sides, sometimes being a 
diagonal, but, in general, an ellipse inscribed in the rectangle. 
Example 2. m = n + h, where h is small. If we write the 
equations in the form : 

x = a cos nt 




(9) 



y = b cos (n + A/ + e) 

then, for the duration of time T 2w/n, 
ht + is nearly constant, and the path is 
FIG. 98 nearly an ellipse which, however, does 

not quite close. And now, in the next in- 
terval of time, the path again will be a near-ellipse, but in a 
slightly different orientation its points of tangency with the 
circumscribing rectangle will be slightly advanced or retarded, 
depending on whether h is positive or negative. 

Thus a succession of near-ellipses will be described, all inscribed 
in the same fixed rectangle x = a, y = 6. The motion can 
be realized approximately experimentally as follows. 

Blackburn's Pendulum. By this is meant the mechanical sys- 
tem that consists of an ordinary pendulum, the upper end of 

* Their directions are determined, in either way, by the formula : 



cos 2* = or cos 2y 



. 
6 2 sin 2e 2ab cos c 

where y denotes the angle from the axis of x to an axis of the conic. The length* 
of the axes are found to be : 



where 

A 8 = a 4 -f 2a*&* cos 2 + b*. 



KINEMATICS IN TWO DIMENSIONS 185 

which is made fast at the mid-point of an inextensible string whose 
two ends are fastened at the same level. When the bob oscillates 
in the vertical plane through the supports, the second string 
remains at rest, and we have simple pendulum motion, the length 
of the pendulum being Z, the length of the first string. 

Secondly, let the bob oscillate in a vertical plane at right angles 
to the line through the points of support, and mid-way between 
these. Again, we have simple pendulum motion ; but the length 
is now I' = I + d, where d denotes the sag in the second string. 
For small oscillations, the coordinates of the bob will evidently 
be given approximately by Equations (3), and by suitably choos- 
ing I and d, we can realize an arbitrary choice of m and n. 

The Sand Tunnel.* If the bob of the pendulum is a tunnel 
of small opening, filled with fine sand, the sand, as it issues from 
the tunnel, will trace out a curve on the floor which shows ad- 
mirably the whole phenomenon of the Lissajou's Curves. In 
particular, if the second string is drawn as taut as is feasible, 
so that d is small, the two periods will be nearly, but not quite, 
equal ; and it is possible to observe the near-ellipses steadily 
advancing, flashing through near-right lines (the diagonals of 
the fixed rectangle). 

Example 3. m 2n. Begin with the case 7 = 0* e = 0, and set 

<p nt: 

(10) x = a cos <p, y = b cos 2<p. 
Hence 

(11) */ = I** - 6 

and the curve is an arc of a parabola, passing through the vertices 
(a, 6), (a, 6) of the circumscribing rectangle and tangent to 
the opposite side at the mid-point. The sand pendulum may 
be released from rest at the point (a, 6), and it then traces re- 
peatedly the parabolic arc. In the general case, 

(12) x = a cos <p, y = A cos 2<p B sin 2<p ; 

A = b cos 6, B = b sin e. 

* This experiment should be shown in the course. It is not necessary to have 
a physical laboratory. A tunnel can be bought at the Five and Ten, and string 
is still available, even in this age of cellophane and gummed paper. 



186 



MECHANICS 



When e is small, the curve runs along near to the parabola; cf. 
Fig. 100. It is symmetric in the axis of y, since ^ and <p' <p + TT 
give x' = x, y' = y. It is tangent once to each of the sides 
x = a, x = a of the circumscribing rectangle, and twice 
to each of the other two. sides. When e has increased to ?r/2, 
A = and 

(13) x = a cos <p, y = b sin 2p 
or 




FIG. 99 



This curve is obtained at once by affine 
transformations from the curve 



(15) y z 

which is readily plotted. 

When c has reached the value TT, we have again an arc of a 
parabola the former arc, turned upside down. As e continues 
to increase, the new curves are the mirrored images of the old in 
the axis of x, for e' = e + TT reverses the signs of A and B. All 
these curves except the arcs of parabolas are quartics, inscribed in 
the fixed rectangle, and having symmetry in the axis of y. 

Example 4. m = 2n + h, where h is small. Here, 

f x = a cos nt 

(16) _ 
I y = b cos [2n* + ht + e] 

and for a single excursion, M is nearly 0. 
Thus the new curve runs along close to an 
old curve for a suitable fixed c, but as time 
elapses, the suitable e advances, too. FIG. 100 

The student can readily trace these curves 

with the sand tunnel. If he does his best to make d = J, there 
will be enough discrepancy to provide for a small h. 

17. Continuation. The General Case. The Commensurable 
Case. Periodicity. Let m and n be commensurable, 




where p and q are natural numbers prime to each other. Then 
n = ap, m = aq. 



KINEMATICS IN TWO DIMENSIONS 187 



(x = a< 
, 
y = b( 



Let <p = at, 7 = 0. Then 

= a cos p<p, 
y = 6 cos (? + e). 

These functions are periodic with the primitive periods 2ir/p 
and 27r/<7, and evidently have the common period 2ir. The 
smallest positive value of co for which 

a cos p(<p + co) = a cos p^> 
6 cos {(/(p + co) + e} = fe cos {</p + e} 
is co = 27T. For, if to is to be a period of the first function, then 

x 2?r 

CO = A 

P 

And if co is to be a period of the second function, then 

27T 

CO = M 

Hence 

X /* . 

- = -, Xg = ,, 

and the smallest values of X, n in natural numbers which satisfy 
this equation arc X = p, n = q. 

From the periodicity of the functions it appears that the curve 
is closed, arid thus, as t increases, the curve is traced out re- 
peatedly. For a non-specialized value of e, the curve is tan- 
gent to each of the sides x = a, a of the circumscribing rec- 
tangle p times, corresponding to the solutions of the equations 
cos p<p 1, 1 ; and q times to each of the sides y 6, 6. 
A line x = x', a < x' < a, cuts the curve in 2p points ; a 
line y = y'j b < y' < 6, in 2q points. 

These curves are all algebraic, and rational, or unicursal. 
For, on setting = tan -J-p, the variables x and y appear, by 
de Moivre's Theorem, as rational functions of . The curves 
are all symmetric in the axis of y. 

The Incommensurable Case. Aperiodic. If on the other hand 
n/m is incommensurable, the curve never closes. It courses 
every region contained within the rectangle. If P be an arbi- 
trary point of the rectangle, the curve will not in general pass 
through P ; but it will come indefinitely near to P not merely 
once, but infinitely often ; possibly, occasionally passing through P. 



188 MECHANICS 

The proof can be given as follows. Consider a circle and the 
angle <p at the centre. Let <f> = = 2wa be an angle which is 
incommensurable with 2?r; i.e. let a be irrational. Then the 
points of the circle which correspond to , 2, 3, (denote 
them by P t , P 2 , ) are all distinct. Hence they must have at 
least one point of condensation, P. But from this follows that 
every point must be a point of condensation. For, let P n and 
P m be two points near P. Then the point corresponding to 
n w must be near the point corresponding to <p = 0. Hav- 
ing thus obtained an arc of arbitrarily small length, we have but 
to take multiples of it, i.e. to construct the points P*( n -m)i 
k = 1, 2, 3, , to come arbitrarily near to any point on the 
circumference. 

Turning now to the equations of the curve, let 

m 

<p = nt, = a. 
n 

Then 

x = a cos <f>, 



1 y = b cos (cup + 17). 
Let a g x' ^ a, and let <p = <p' be a root of the equation 

x f a cos <p. 
The curve cuts the line x = x' in the points for which 

y = b cos {<*(<?' + 2kw) + r?}, 6 cos {(- <?' + 2kw) + y}. 

And now, since the angles 2kair lead to points on the circle which 
are everywhere dense, the corresponding values of the cosine 
factor are also everywhere dense between 1 and + 1. 

It is of interest to study the multiple points of the curve. These 
occur when 

t) <f>' = kw + 1 ^, I ^0; 

it) ^ = )br + ^~a' fc?0; 

provided 

(19) -n * (1 + k a)ir. 

When the inequality (19) holds, there is a one-to-one cor- 
respondence between the values of <p and the points of the curve, 



KINEMATICS IN TWO DIMENSIONS 189 

provided the multiple points (which are always double points 
with distinct tangents) are counted multiply. If, however, 

(20) 77 = (1 + k Q a)7r, 

then 

a<p + f\ = a (<p + fc 7r) + i 7r. 
Set 

(21) = <f> + k Q w. 
Then the Equations (18) become : 

x = a! cos 



<22> I = 

where a! = a or a, and likewise &' = 6 or 6. Let 

^ < oo. 

Then there is a one-to-one correspondence between the values 
of 6 arid the points on the curve. The point for which 9 = : 

x = a', y = &', 

is an end-point of the curve. It is simple, no other branch going 
through it. The double points correspond to the values 

0' = kw + - > 0, 
a 

where 

/CTT - - > 0, I ^ ; 
a. 

or where 

- far + - > 0, k ^ 0. 



and n-Dimensions. In the case of motion with three 
degrees of freedom, the equations can be reduced to the form : 



(23) 



x a cos <p 

y = b cos (ay + ??) 

z = c cos ($v + f ) 



The case that a, /3 are both commensurable can be discussed as 
before. The curve closes, the motion is periodic. When a 
and ft are both irrational, and their ratio is also irrational, it can 



190 MECHANICS 

happen that the curve courses every region, however small, of 
the parallelepiped : 

a^xga, 6^2/^6, c ^ z ^ c, 

and has no multiple points, the correspondence between the 
points of the curve and the values of <p when oo < <p < oo 
being one-to-one without exception Whether the former prop- 
erty is present for all such values of a and 0, provided further- 
more that or, /3, and /3/a are not connected by a linear non-homo- 
geneous equation with integral coefficients, and that 77, J" are not 
specialized, I cannot say, though I surmise it to be. The latter 
property, however, can be established. 
The same statements hold in the general case, 

x k = a k cos (oL k <p + rik), k = 1, - - , n. 

If; may happen, in a dynamical system with n degrees of free- 
dom and coordinates q lt , q n , that only a sub-set, <ft, , 
q m , 1 g m < n, execute a Lissajou's motion. Thus a Black- 
burn's Pendulum suspended in a moving elevator will have its 
projection on a horizontal plane executing a Lissajou's motion, 
whereas the vertical motion is not periodic at all. 

The late Professor Wallace Clement Sabine drew mechanically 
some very beautiful curves, which are here reproduced in half-tone. 
I still have the half-tone which Dr. Sabine gave me. So far as I 
have been able to ascertain, the curves were never published. The 
figures here shown were made from lantern slides in possession of 
the Jefferson Physical Laboratory, and it is through the courtesy of 
the Laboratory that I have been enabled to reproduce them here. 



CHAPTER VI 
ROTATION 

1. Moments of Inertia. The moment of inertia of n particles, 
w,-, with respect to an axis is defined as the sum : 

(1) / = i><r<, 

<=i 

whore r denotes the distance of w t - from the axis; cf. Chapter 
IV, 10. 

Let be an arbitrary point of space, and let Cartesian axes 
with as origin be assumed. Let the moments of inertia about 
the axes be denoted as follows : 



(2) 



A = 



The products of inertia are defined as the sums : 
(3) -0 = 5 m i Vi z <> E = 



These definitions are extended in the usual way by the methods 
of the calculus to continuous distributions. 

In terms of the above six constants it is possible to express 
the moment of inertia about an arbitrary axis through 0. Let 
the direction cosines of the axis be a, 0, y and let P : (x, y, z) 
be an arbitrary point in space. Then 

r 2 = p2 _ <^ 

or 

r 2 = x 2 + tf + z 2 - (ax + py + yz) 2 . 
Since o p 

of + P + 7 2 = 1, FlG - 

the last expression for r 2 can be written in the form : 

(x 2 + 2/ 2 + * 2 )( 2 + P + 7 2 ) - (ox + fry + yz)*. 

191 




192 MECHANICS 

Hence 



- 2yazx - 
Thus 

/ = a 2 5) m;(^ 2 + z> 2 ) + 2 5J m t -(*i 2 + a* 2 ) + etc. 
or: 

(4) 7 = 4a 2 + 50 2 + CV - 2D07 ~ 2#y - 2Fa/3. 

This is the desired result. The meaning of the formula can 
be illustrated by the Ellipsoid of Inertia. Consider the quadric 
surface, 

(5) Ax 2 + By 2 + Cz* - 2Dyz - 2Ezx - 2Fxy = 1. 

It is known as the Ellipsoid of Inertia, and its use is as follows. 
Let an arbitrary line through with the direction cosines , 0, 7 
meet the surface in the point (X, Y, Z), and let p be the length 
of the segment of the axis included between the centre of the 
ellipsoid and its surface. Then 

X = ap, Y = 0p, Z = yp. 
Since X, Y, Z satisfy (5), it follows that 

(6) p 2 (^la 2 + Bp + C7 2 - 2D/37 - 2#ya - 2Fa/3) = 1. 
On combining (4) and (6) we find : 

(7) P 2 / = 1, / = ^ 

and / is seen to be the square of the reciprocal of p. From this 
property it appears that the Ellipsoid of Inertia is invariant of 
the choice of the coordinate axes. 

If all n particles m z lie on a line, Equation (5) no longer repre- 
sents an ellipsoid. Let the axis of z be taken along this line. 
Then A = B and all the other coefficients vanish. Thus (4) be- 

comes 7 = 4 (' + *). 

Here, A ^ except in the single case that i = 1 and m l lies at 
the origin. In all cases but this one, the quadric surface (5) 
still exists, being the cylinder of revolution 

(8) A(* 2 + 2/ 2 ) = 1, 
and the theorem embodied in (7) is still true. 



ROTATION 193 

Suppose, conversely, that (5) fails to represent a true (i.e. 
non-degenerate) ellipsoid. If all the coefficients A, B, , 
F are 0, the system of particles evidently reduces to a single 
particle situated at 0. In all other cases, (5) represents a central 
quadric surface, S. If this is not a true ellipsoid, then there is 
a line, L, which meets 8 at infinity; i.e. which does not meet S 
in any proper point, but is such that a suitably chosen variable 
line L' always meets S, the points of intersection receding in- 
definitely as L f approaches L. The moment of inertia about 
L' is given by (7) and approaches as L' approaches L. Hence 
the moment of inertia about L is 0. But if the moment of inertia 
of a system of particles about a given axis is 0, it is obvious that 
all the particles must lie on this axis. 

We see, then, that (5) represents a true ellipsoid in all cases 
except the one in which the particles lie on a line, and that (7) 
holds in all the latter cases, too, except the one in which the 
system reduces to a single particle situated at 0. 

Parallel Axes. We recall, finally, the theorem relative to par- 
allel axes ; Chapter IV, 10 : 

THEOREM. The moment of inertia, I, about any axis, L, is 
equal to the moment of inertia, 7 , about a parallel axis, L , through 
the centre of gravity, plus the total mass times the square of the dis- 
tance, h, between the axes: 

I = J + MW. 

EXERCISE 

Show that the moment of inertia about any line, L, in space 
is given by the formula : 

7 = {A + M(y\ + *?)} a 2 + {B + M(z\ + x$\ /3 2 
+ {C + M(x\ + tf)} 7 2 - 2(Z> + M Vl zJ 0y 
- 2(E + MZ.X,) ya - 2(F + Mx.y,) aft 

where the origin of coordinates is at the centre of gravity and 
x \> y\j z \ arc ^ ie coordinates of any point on L, and where a, ft y 
are the direction cosines of L. 
For an arbitrary system of axes, replace x lt y ly z l respectively by 

*i ~ *> y\ - y> *i - *> 



194 MECHANICS 

where #, ?/, 2 are the coordinates of the centre of gravity, and 
x u Vn z \ are the coordinates of any point on L all referred to 
the new axes. 

2. Principal Axes of a Central Quadric. Let a quadric surface 
be given by the equation : 

(1) Ax 2 + By* + Cz* + 2/)7/* + 2Ezx + 2Fxy = 1, 

where the coefficients are arbitiary subject to the sole restriction 
that they shall not all vanish. The problem is, so to rotate the 
axes that the new equation contains only the square terms. Let 

(2) F(x, y, z) = Ax 2 + Eif + Cz* + 2Dyz + 2Ezx + 2Fxy, 

(3) *(*, P,s) = x* + y* + z*. 

Consider the value of the function F(x, y, z) on the surface 
of the sphere 

(4) ' x* + ?/ 2 + z 2 = a 2 , or *(x, y, z) = a 2 . 

Since F(x, y, z) is continuous and the sphere is a closed surface, 
the function must attain a maximum value there, and also a 
minimum. 

Let the axes be so rotated that the maximum value is assumed 
on the axis of z } in the point (0, 0, f), where f = a. We think 
of Equations (2) and (3) now as referring to the new axes. 

In accordance with the Method of Lagrange * we form the 
function 

F + \$, 

the independent variables being x, y, z, with X as a parameter ; 
and we then sot each of tho first partial derivatives equal to : 

(5) b\ + X*, = 0, F 2 + X$ 2 = 0, t\ + X$ 3 = 0. 

These three equations, combined with (4), form a necessary 
condition on the four unknowns x, y> Zj X for a maximum : 

' Ax + Fy + Ez + \x = 

(6) Fx + By + Dz + \y = 
Ex + Dy + Cz + \z = 

But we know that the point (0, 0, f), f ^ 0, yields a maximum. 
Hence D = 0, E = 0, 

* Lagrange's Multipliers, Advanced Calculus, Chapter VII, 5. 



ROTATION 195 

and the new F(x, y, z) has the form : 

. F(x, y, z) = Ax* + 2Fxy + By* + Cz\ 
If the coefficient of the term in xy does not vanish, it can be 
made to do so by a suitable rotation of the axes about the axis 
of z; cf. Analytic Geometry, Chap. XII, 2. Thus F(x,y,z) is 
reduced finally by at most two rotations (these may be combined 
into a single rotation, but that is unessential) to the desired form : 

(7) F(x, y, z) = Ax* + By* + Cz\ 

Here, A, B, C may be any three numbers, positive, negative, 
or 0, except that we have excluded as trivial the case that 
all three vanish. The original equation (1) will obviously repre- 
sent an ellipsoid if and only if the new coefficients A, B, C in (7) 
are all positive. We have thus established the following theorem. 

THEOREM. An arbitrary homogeneous quadratic function 
F(x, y, z) can be reduced by a suitable rotation of the axes of coordi- 
nates to a sum of squares. The new coefficients of x r , y', z 1 may 
be any numbers, positive, negative, or 0. 

EXERCISE 

Show, by the method of mathematical induction and La- 
grange's Multipliers, that an arbitrary homogeneous quadratic 
function in n variables, 



can be reduced to a sum of squares by a suitable rotation. 
By a rotation is meant a linear transformation : 
x{ = a n x 1 + + ai n x n 



x' n = a n i#i + + a nn x n 



such that, for any two corresponding points (x lt , x n ) and 
(x( 9 , x' n ), the relation holds : 

r '2 _L . . . 4. r '2 r 2 J_ . . . 4. r 2 
*l \ \ *n ~ *\ \ \ An ) 

and the determinant of the transformation, 
A = S a n a nn , 
which necessarily has the value 1, is equal to + 1. 



196 MECHANICS 

It is easy to write down the conditions that must hold between 
the coefficients of the transformation, but these conditions are 
not needed for our present purpose. Obviously, the result of 
any two rotations is a rotation. 

3. Continuation. Determination of the Axes. In the fore- 
going paragraph we have been content to show the existence of 
at least one rotation, whereby the given function is reduced 
to a sum of squares. We have not computed the values of the 
new coefficients, nor have we determined the lengths of tho axes. 
Now, any rotation of the axes carries the second function, $, over 
into itself : 

*'(*', */', z') s *(*', ', z') = *(x, y, z). 

The function : 

fl = F + \3>, 

goes over into the function : 

F' + X*', 
where X remains unchanged. Now, the condition : 



an _ 00 

~ ' ~ ' 



a? ~ ' 

is equivalent to the condition : 



since the determinant of the linear transformation does not 
vanish. Hence Equations (6) of the preceding paragraph will 
be of the same form for the transformed functions. When 

F'(x', y', *') = A'x'* + B'y'* + C'z">, 
the equation for determining X reduces to the following : 

(A' + X)(B' + X)(C" + X) = 0. 
Thus the three roots of the determinant of Equations (6), 

A +\ F E 

(8) As F B + \ D 

E D C + 



ROTATION 197 

arc seen to be the negatives of the coefficients A', B' t C', and so 
the axes of the quadric are found. If the roots of the deter- 
minant (8) are denoted by \ 19 X 2 , X 3 , the lengths of the semi- 
axes are 



In case a X = 0, the quadric reduces to a cylinder, or more spe- 
cially, to two planes. All three X's will vanish if and only if the 
original F(x, y, z) vanishes identically. 

When tho X t have once been determined, Equations (6) give 
the equations of the axes of the quadric. In general, the three 
\i are distinct, and Equations (6) then represent a right line 
for each X. 

4. Moment of Momentum. Moment of a Localized Vector. 

Let A be a vector whose initial point, P, is given, and let be 
any point of space. Let r be the vector drawn from to P. 
By the moment of A with respect to is meant the vector, or outer 
product : * 

(1) r X A. 

We have met this idea in Statics, where the moment of a force 
F, acting at a point P, with respect to a point was defined as 
the vector 

M = r X F. 

The moment of momentum of a particle with respect to a point is 
defined as the vector | 

(2) ff = r X mv, 

whore r is the vector drawn from the point to 

the particle, and v is the vector velocity of the FIG. 102 

particle. 

The moment of momentum of a system of particles with respect 
to a point is defined as the vector 

n 

(3) ff = J) r k X m k v k , 

1=1 

* Cf. Appendix A. 

f Contrary to tho usual notation of writing vectors in boldface, as a, x, i, 
etc., or by parentheses, as (co), it seems here expedient to denote the vector moment 
of momentum by a, the vector momentum by p, and the vector angular velocity 
by o>. 




198 



MECHANICS 



where r k is drawn from the point in question to nik, and v^ is tin 
vector velocity of m,k. 

In the case of a continuous distribution of matter the extensioi 
of the definition is made in the usual way by definite integrals. 

In Cartesian form a has the value, for a single particle : 



(4) 



J 1 

y - 

dy 

'dt m dt m dt 



dx 



dz 



dz di 



dx 



dz 



dx 



the origin being at 0. And so, for a system of particles, th( 
components of a along the axes are : 



(5) 



Rate of Change of <r. Since 

(&} *L ( ^y. _ di 

dt \ dt dt 
it is seen from Equations (5) that 



(7) 



dx k dz 



dx 



d z x 

- y-^~v 



These equations, in vector form, become : 

(8) ljt = ^ mkTk X a *' 

where a^ denotes the vector acceleration of the fc-th particle. 



ROTATION 199 

The result, Equation (8), could have been obtained at once 
from (3). If we differentiate Equation (2), we find : 

da ^, dv . di ^, 

_ = mrx __ + w ._* xv . 

Now, 

-77 = v and v X v = 0. 
at 

Hence 

do- . y dv 

dt = mr X dt = r * a > 

where a denotes the vector acceleration. Similarly, from (3) 
we derive (8). 

5. The Fundamental Theorem of Moments. In Chap. IV, 
3, it was shown that, in the case of any system of particles in a 
plane such that the internal forces between any two particles 
are equal and opposite and lie along the lino through the particles, 
the moments of the internal forces annul each other, and the 
equation of rotation becomes : 

(1) I; m k (x k ^ - y k d ji*) = 2 ( Xk Y 



k 

fc= 1 



The theorem and its proof can be generalized at once to space 
of three dimensions. Newton's Second Law of Motion is ex- 
pressed for the particle m k by the equations 

d*Xk _ v _i_ 

'<~W~ Xk + 

J 

= Y k + X Y 



where F*/ denotes the internal force which is exerted on the 
particle w* from the particle my. Multiplying the third of these 
equations by y^ the second by z k and adding, and observing 
that the moments of the internal force cancel in pairs, since the 
forces F/jfc and F*/ are equal and opposite and have the same line 
of action, the first of the following three equations is obtained. 
The other two are deduced in a similar manner. 



200 MECHANICS 



(2) 



These equations express the Fundamental Theorem of Mo- 
ments. In vector form it is : 

(3) S-i>XF, 
or: 

^7 = 2) (Moments of the Applied Forces about 0). 

Equation (3) can be deduced more simply by vector methods. 
Write Newton's Second Law in the vector form : 

(4) m k a k = F* + 2) F w . 
Next, form the vector product, 

(5) m k T k X a* = r fc X F* + 2) r * X F*/, 

and add. The sum on the left is equal to d<r/dt by 4, (8). On 
the right, the vector moments of the internal forces cancel in 
pairs, and there remains the right-hand side of (3). 

FUNDAMENTAL THEOREM OF MOMENTS. The rate of change 
of the vector moment of momentum of any system of particles is 
equal to the vector moment of the applied forces, provided that the 
internal forces between each pair of particles are equal and opposite 
and in the line through the particles : 



or, in Cartesian form t Equations (2). 

The foregoing result applies to the most general system of 
particles, subject merely to internal forces of the very general 
nature indicated. By the usual physical postulate of continuity 
we extend the theorem to the case of continuous distributions 



ROTATION 201 

of matter, or to any material point set. For example, our solar 
system is a case in point, and we will speak of it in detail in 7. 

6. Vector Form for the Motion of the Centre of Mass. Let 

be an arbitrary fixed point in space, and let f be the vector drawn 
from to the centre of gravity, (?, of a material system. Let 
Fi, , F n be the forces that act; i.e. the applied, or external, 
forces. Then the Principle of the Motion of the Centre of Mass 
is expressed by the equation : 



(1) M - 



., 



where v = df/dt. Equation (1) is merely the vector form of 
Equations A), Chapter IV, 1. It can be derived by vector 
methods, by adding Equations (4), 5, and observing that 

Mi = 2) 

= 1 

Let p denote the momentum, 

p = M v. 
Equation (1) now takes on the form : 

(2) 

Thus we have for any system of particles, rigid or deformable, 
and even for rigid bodies and fluids, the two equations of momen- 
tum : 

THE EQUATION OF LINEAR MOMENTUM : 
A) \ 

THE EQUATION OF MOMENT OF MOMENTUM : 

7. The Invariable Line and Plane. In case no external forces 
act, 

< a - " 



202 MECHANICS 

and the vector cr remains constant. The line through collinear 
with <T is called the invariable line with respect to 0, and a plane 
perpendicular to it, the invariable plane with respect to 0. 

The solar system is a case in point, if we may neglect any force 
the stars may exert. We may consider the actual distribution 
of matter and velocities, and then, on choosing a fixed point, 
0, the corresponding value of a will be constant. 

Or we may replace the sun and each planet by an equal mass 
concentrated at its centre of gravity, and consider this system. 
Again, the vector a- corresponding to a given point will be 
constant, and obviously nearly equal to the former a. 

Let us choose one of these cases arbitrarily and discuss it further. 
The vector a depends on the choice of 0. Can we normalize 
this choice? The centre of mass of the solar system is not at 
rest, and so, since we are neglecting any force exerted by the 
stars*, the momentum of the system, p = Mv, is constant and 
5^ 0. The direction of this vector, p or v, does not depend on 
the choice of 0. The point 0' can be so chosen that a' is collinear 
with p. 

We shall show in the next paragraph, Equation (5), that 

(2) a = a' + Mr X V, 

where a, a' are referred to 0, 0' respectively. If a is not already 
collinear with p, let <r be resolved into two components; one, 
collinear with p, the other, cr , at right angles. We wish, then, 
so to determine r that 

(3) Mr Q X v = (7 , <T O * 0. 

Since o- and v arc perpendicular to each other, this can be done. 
The point O f will be any point of a line collinear with p. This 
is known as the invariable line of the solar system. For a further 
discussion, cf. Routh, Rigid Dynamics, Vol. I, p. 242. 

8. Transformation of <r. Let be a point fixed in space, 
p and let O' be a second point, moving or fixed. Let 
P be the position of a particle of the system. Then 



o r CD f r = r' + r ; 

Fia. 103 I V = v' + V , 

where v' expresses the velocity of P relative to 0', and V is the 
velocity of 0' . 



ROTATION 203 

For a single particle, the moment of momentum with respect 
to is the vector 

<r = r X rav = mr' X (v' + v ) + mr X v, 
or 

(2) <r = mr' X v ; + mr X v + mr' X v . 

The first term on the right has the value 

a' r = r' X wv', 

or the relative moment of momentum, referred to 0' as a moving 
point. 

For a system of particles we infer that 

* x v * 



or 

(3) <r = <r' r + Mr X v + Mi' X v , 

where o> is the relative moment of momentum referred to 0' as 
a moving point ; v is the velocity of the centre of mass ; and f ' 
is the vector drawn from 0' to the centre of mass. 
The second term on the right, 

Mr X v = r X Mv, 

can be interpreted as the moment of momentum, relative to O, 
of the total momentum, Mv, of the system, thought of as a mass, 
M , concentrated at O 1 and moving with the velocity v. 
The third term, 

Mr' X V = f' X Mv , 

is the moment of momentum, relative to 0', of the total mass, 
M j concentrated at the centre of gravity and moving with ve- 
locity V . 

If, in particular, 0' be taken at (?, then f' = 0, v = v, and 

(4) <r = <r' r + Mr X v, 

where o> denotes the relative moment of momentum, referred 
to G as a moving point, and 

Mr X v = f X Mv 

is the moment of momentum, Mv, of the total mass, concentrated 
at G and moving with the velocity of G, referred to 0. 



204 MECHANICS 

Let cr' denote the value of a referred to the point 0' as a fixed 
point; i.e. 

X v k . 



Then 

</ = 5J m ^i X vi + ] m k ri X v 

or 

</ = v'r + Mr' X v . 

Thus Equation (3) goes over into : 

(5) a = </ + Mr X v. 

This amounts to setting v = in (3). 

9. Moments about the Centre of Mass. We have the Funda- 
mental Equation of Moments, 5 : 

(I)' S 

And we have the Equation of Transformation, 8, (4) : 
(2) a = *' r + Mf X v, 

where o> is the relative moment of momentum, referred to G as 
a moving point. 

Differentiate this last equation, observing that 



since df/dt = v is cither or else collinear with v. Thus we find : 

/ON da _ dff'r M d? 

(6) dt ~ Ht + M X Tt 

On the other hand, 

r = r' + f , 

where r, f are drawn from ; r' from 0. Thus 
(4) 5) r* X F = g r; X F* + f X 5) F*. 

t k Ic 

Substituting in Equation (1) the values found in Equations (3) 
and (4), we obtain the result : 



ROTATION 205 

Recall the Equation of the Motion of the Centre of Mass, 6 : 

(6) " 

From it follows that 

Mr X ^ = f X F*. 

fc 

Thus these terms cancel in (5) and there remains : 



In this equation is embodied the result which may be described 
as the 

PRINCIPLE OF MOMENTS WITH RESPECT TO THE CENTRE OF 
MASS. The rate of change of the relative vector moment of momen- 
tum, referred to the centre of mass G regarded as a moving point, 
is equal to the sum of the vector moments of the applied forces with 
respect to G: 



EXERCISE 

Show that a rigid body is dynamically equivalent, in general, 
to a pair of equal masses on the axis of or, a second pair on the 
axis of y, and a third pair on the axis of z, each pair being situ- 
ated symmetrically with respect to the origin, and all six dis- 
tances from the origin being the same ; it being assumed that the 
principal axes of inertia lie along the coordinate axes. Discuss 
the exceptional cases. Use the results of 12. 

10. Moments about an Arbitrary Point. Consider the most 
general transformation, 8, (3) : 

(1) * = <j' T + Mr X v + Mr' X v , 

and differentiate : 



On the other hand, 

(3) 2 r " x F * = 2 r i x F * 

t I 



206 MECHANICS 

From the Equation of Linear Momentum, 6, (1) follows that 

(4) MI O X % - 2 r o x F *- 

G/v ^^T 

Moreover, 

-jj V -f- V - . 

For, 

hence 

v X v = v X v' + v X v = v X v', 
and 

v X v' + v' X v = 0. 

Substituting, then, in the Equation of Moment of Momentum, 
6, B): 

g = 2r*XF*, 
t 

and reducing, we find : 



This equation is general, covering all cases of taking moments 
about a moving point 0', relative to that point. When, however, 
one uses the expression: " taking moments about a point O'" 
the meaning ordinarily attached to these words is, that the equa- 
tion 

(6) f = ? r i>< F * 
shall be true. Hence we must have 

(7) f 'X = 
for every value of t. 

Let t = T be an arbitrary instant. Let 0' be a point which 
describes a certain path, 

(8) r - r ft r). 

Consider this as the vector r of the foregoing treatment. Then 



ROTATION 207 

At the instant t = r, 

/ dv *\ / a2f <A 

(-5-),., = (IF;,.; 

Then Equation (7) is to hold for this vector r at the one instant 
t = T. 

Thus we have in general, not a single curve traced out by 0' 
and (7) considered for a variable point of that curve, as in the 
case of 8, where f' = 0, but a one-parameter family of 
curves, and Equation (7) considered for one point of each curve ; 
cf. for example, the next paragraph. 

11. Moments about the Instantaneous Centre. Consider the 
motion of a lamina, i.e. a rigid plane system, in its own plane. 
Let Q be the instantaneous centre at a given instant, t = T. 
Then <r, referred to the point Q, is a vector perpendicular to the 
plane, and its length is 

T de 

1 dt' 

where / is the moment of inertia of the lamina about Q. 
What does it mean to "take moments about Q"? From the 
foregoing it means to take moments about a point 0' describing 
a curve 

TO = *o& T) 

which at the instant t = r passes through Q. 

There is an unlimited set of such curves. Let us select, in par- 
ticular, the curve C which is the path of that point fixed in the 
lamina, which passes through Q at the instant t = r. Observe 
that this is an arbitrary choice of C. This curve C is known in 
terms of the rolling of the body centrode on the space centrode. 
The velocity of 0' at Q is 0, but its acceleration, if Q is an 
ordinary point, is normal to the centrodes at Q and does not vanish ; 
Chapter V, 5. If, then, Equation (7), 10 is to be satisfied, the 
centre of gravity, G, must lie in the normal to the centrodes. In 
particular, the normal to the body centrode must pass through 
the centre of gravity. Hence the body centrode must be a circle 
with the centre of gravity at the centre, if the condition is to be 
permanently satisfied. The equation of moments now becomes : 

I-JJ2 ~ S (Moments about Inst. Centre). 



208 MECHANICS 

The only case, then, of motion in a plane, in which we may 
permanently take moments about the instantaneous centre, 
thought of as a point fixed in the moving body, is that in which 
a circle rolls on an arbitrary curve, the centre of gravity being 
at the centre of the circle; and the limiting case, namely, that 
the point Q is permanently at rest. This last case corresponds 
to the identical vanishing of dvjdt. 

Moments about an Arbitrary Point. Consider now an arbi- 
trary point 0' fixed in the body. Let it be at Q at the instant 
t = r, and let C be the curve, 

TO = r (J, T), 
which it is describing. Take moments about Q with reference 

to this point, 0'. Then 

da[ = d?0 
dt dt 2 ' 

If, furthermore, Equation (7), 10 is satisfied, the equation of 
moments becomes : 

/-72/) 

^77/2" = 2} (Moments about Q). 

Equation (7) here means, in general, that the acceleration of 0' 
is collinear with the line determined by Q and G. In particular, 
the equation is satisfied if the acceleration of O' is at Q ; or if 
Q coincides with G. * 

EXERCISE 

A billiard ball is struck full by the cue. Consider the motion 
while there is slipping. Show that it is not possible to take 
moments about the instantaneous centre. 

Find the points of zero acceleration and verify the fact that 
it is possible to take moments about them, explaining carefully 
what you mean by these words. 

Show that the points whose acceleration passes through the 
centre of the ball lie on a circle through the centre of the ball, 
of radius one-fifth that of the ball, the centre being directly above 
the centre of the ball. 

12. Evaluation of <r for a Rigid System; One Point Fixed. 

Consider a rigid system of particles with one point, 0, fixed. 

* Ed ward V. Huntington has discussed this question, Amer. Math. Monthly, 
vol. XXI (1914) p. 315. 



ROTATION 



209 



The motion is then one of rotation about an axis passing through 
] cf . Chapter V, 8. Let the vector angular velocity be 
denoted by w, and let a, p, 7 be a system of mutually perpen- 
dicular unit vectors lying along Cartesian axes with the origin 
at 0. When we wish these axes to be fixed, we shall use the 
coordinates (x, y y z) and replace QJ, j3, 7 by i, j, k. In the general 
case, the coordinates shall be , 17, f . 

Let P be any point fixed in the body, and let r be the vector 
drawn from to P : 



a) 

The velocity of P, 
(2) 



r = $ + lift + f y. 



" 



is expressed in terms of the vector co as follows (Chapter V, 9) : 

(3) v = co X r. 
In Cartesian form, 

(4) v = 



or 



(5) 



For a single particle, then, a has the value : 
(6) a = r X rav, 



(7) 



Hence 



(8) 



a = m 



y 

r 



210 MECHANICS 

These formulas lead in turn to the following : 

<T = m [(rj* + f 2 ) C0 - &CO,, - 



(9) 



= m [ - rft + (f 



= m [ - fcof - ftw, + ( 2 + i; 2 



For a system of particles they become : 






and so, finally, 

(10) 



or = - 



These are the formulas which give the components of a along 
the axes of , 77, f when the origin is fixed. It is obviously im- 
material whether the axes are fixed or moving. 

13. Euler's Dynamical Equations. Consider the case of a 
rigid body, one point of which is fixed. The Equation of 
Moments, 

(1) -rr = 2 ( Moments about ), 

referred to this point, admits a simple expression in terms of the 
angular velocity, &, of the body. Let the (, r/, f)-axes be fixed 
in the body, and let P be a point which moves according to any 
law. Let 

r = <* + T70 + f% 

where r is the vector drawn from to P. Then we have seen 
(Chapter V, 14) : 

dr = 

dt 



This result applies to the vector : 

o- = cr$ a + (Ty 13 + <TS 7, 
and thus gives us the left-hand side of (1). 



ROTATION 
On the right-hand side of (1) let 

X F* = La + M/3 + Ny. 



211 



Thus we have : 



(2) 



= L, 



dt 

dt 
dfft -LJ 

~ _j." | C0 O"TJ WTJ (7A == xV. 

at 

On substituting for <T, o^,, a^ their values from (10), 12, the 
equations known as Euler's Dynamical Equations result. In 
particular, if the (, 77, f)-axes are laid along the principal axes 
of inertia, then 



and Equations (2) assume the form : 

dp 

/j - 

(3) 



where 



P = 



r = 



When the axes of coordinates do not coincide with the prin- 
cipal axes of inertia, Euler's Equations take the general form : 



(4) 

1 



dt 



dt 



dt 



- (En, - 



(C - B) w^ = L, 



and two others obtained by advancing the letters cyclically. 

Eider's Dynamical Equations also apply to the rotation of 
a rigid body about its centre of mass ; 9. Here, there is no 
restriction whatsoever on the motion. 



212 



MECHANICS 



14. Motion about a Fixed Point. Let the body move under 
the action of no forces, save the reaction at 0. Then Euler's 
Equations become the following : 






A first integral is obtained by multiplying the equations re- 
spectively by p, q, and r, and adding : 



(2) 



Ap* + Bq* + Cr* = h. 



This is the Equation of Energy, Chapter VII, 5, 6. 

A second integral is found by multiplying Equations (1) re- 
spectively by Ap, Bq, and Cr, and adding : 

dr 



(3) A 2 p 2 + B 2 q 2 + C 2 r 2 = I 

This equation corresponds to the fact that 



dt 



= 0, 



and so 

a = Apa + Bqf$ + Cry 
is constant. 

From Equations (2) and (3), two of the variables, as p 2 and 
# 2 , can, in general, be determined in terms of the third, and then, 
on substituting in the third equation (1), a differential equation 
for r alone is found. It is seen that t is expressed as an elliptic 
integral of the first kind in r. Thus, p, q t and r are found as 
functions of t. 

Exercise. Let A = 3, B = 2, C = 1 ; and let p, q, r all have 
the initial value 1. Work out the value of t in terms of the in- 
tegral. 



ROTATION 213 

The Body Cone. On multiplying (2) by Z, (3) by A, and sub- 
tracting, we find : 

(4) A(l- Ah) p* + B(l- Bh) g 2 + C(l - Ch) r 2 = 0. 
The equations of the instantaneous axis are : 

(5) -* = ? = , 

' p q r' 

when p, q, r are the above functions of t. Hence the locus of 
the instantaneous axis in the body is the quadric cone : 

(6) A(l- Ah) ? + B(l- Bh) T, 2 + C(l - Ch) f 2 = 0. 

More explicitly, let p, q, r satisfy (2) and (3) and hence (4). 
Then any point (, ry, f) of (5) satisfies (6), and hence lies on 
the quadric cone. Conversely, let (, 77, f) be a point of the 
quadric cone, (6). If (, TJ, f) ^ (0, 0, 0), determine p, q, r, p 
by the four equations 

P = /*> Q = M, r = /if, 



Thus (3) is satisfied. And (4) holds, too. Hence (2) is true. 
Consequently, (, r/, f ) lies on an instantaneous axis. 

The Space Cone. Poinsot obtained an elegant determination 
of the space centrode. Consider the ellipsoid of inertia, 2. It 
is a surface fixed in the body. Let m 
be the point in which the ray drawn 
from and collinear with co cuts S. 
Then the tangent plane M to S at m is 
a plane fixed in space, the same for all 
points, m. The motion is seen to be one 
of rolling of the surface S on the plane 
M without slipping. p IG ^4 

To prove the first statement, it is 

sufficient to show that the tangent plane at m is perpendicular to 
cr, and that its distance from O does not depend on m. The 
equation of S is : 
S: 4 2 + 5T; 2 + Cf 2 = 1. 

The coordinates of m are : 

PP, PQ, pr, where 




214 MECHANICS 

Hence the equation of M is 

M : P Ap^ + pBqv + pCrf = 1. 

The direction components of its normal are Ap, Bq, Cr. But 
these are precisely the projections of <r on the axes. Hence M 
is perpendicular to a. Moreover, the distance of the plane M 
from is 

1 = 1 = J h 

P^l * l ' 



and so is constant. This completes the proof of the first state- 
ment. 

To prove the second statement; consider so much of the body 
cone, (6), as lies in S. Let F be the curve on S which marks 
the intersection of these two surfaces. Then F rolls on M with- 
oujb slipping, and the curve of contact, C, can servo as a directrix 
of the space centrode. For the body cone, (6), rolls without 
slipping on the space cone, and the curves F, C are two curves 
on these cones, which curves aro always tangent at the point M 
of the instantaneous axis. The angular velocity, w, is propor- 
tional to the distance Om ; for 



15. Euler's Geometrical Equations. Euler introduced as co- 
ordinates describing the position of a rigid body, ono point 
of which is fixed at 0, the three angles, 6, p, and ^ represented 
in the figure. Between the components of the angular velocity 
w about the instantaneous axis, 



and these coordinates and their derivatives, exist the following 
relations : 

d$ , dd 

V = Sin COS <p rr + SHI (p -r. 

dt at 



... <ty , de 

q = sin sin ip-j- + cos tp-r 

(it Ctt 



(1) 



dt ' dt 
These are known as Enter' s Geometrical Equations. 



ROTATION 



215 



A geometrical proof can be given by computing the vector 
velocities of certain suitably chosen points in two ways. Begin 




FIG. 105 

with the point C in which the positive axis of f pierces the surface 
of the unit sphere. As we look down on the sphere from above 
this point, it is evident from the figure that 



dO 
dt 



= p sin <p + q cos <p 



sin 6 - = p cos <p + q sin <p. 
(it 




FIG. 106 



These equations yield the first two of Equations (1). 

To obtain the third equation, consider the motion of E. Its 
velocity is made up of a velocity o> tangent to the arc EA, and 
two velocities perpendicular to this arc. On the other hand, 
its velocity is composed of the velocity tp tangent to the arc EA ; 
the velocity \ft cos 0, also tangent to EA ; and perpendicular 
to EA. Hence 



and this is the third Equation (1). 



216 



MECHANICS 



If p, <7, r have onc6" been determined as functions of the time, 
Equations (1) yield a system of three simultaneous differential 
equations of the first order for determining 0, <p, $ as functions 
of the time. Thus in the problem of 14, the motion of a 
rigid body under no forces, or acted on by the one force of con- 
straint that holds the point O fixed, p, q, r were determined 
explicitly as functions of the time, and the further study of the 
problem is based on the above Equations (1). 

16. Continuation. The Direction Cosines of the Moving Axes. 

The moving axes are related to the fixed axes by the scheme, 

V f 



y 

z 

and the question is, to express the nine direction cosines in terms 
of the Eulerian angles. This can be done conveniently by vector 
methods, if we effect the displacement one step at a time. Let 
i, j, k be unit vectors along the original axes, and a, /ft, 7 unit 
vectors along the displaced axes. Let the first displacement 
be a rotation about the axis of z through the angle ^, and let 
i, j go over into i 1; jj. Then 

i t = i cos ^ + j sin ^ 
J! = i sin ^ + j cos ^ 
k k 

*V| JEL. 

Next, rotate about the axis of j t through an angle 6, whereby 
i x goes into i 2 , and k x into k 2 = 7 : 

1 2 = i t cos k t sin 

J 2 = Ji 

k 2 = ij sin + kj cos 6. 

Finally, rotate about k 2 through an angle ^, whereby i 2 goes 
over into i 3 = a and J 2 goes into j 3 = : 

1 3 = i 2 cos <p + J2 sin <p 

j 3 = i 2 sin <p + j 2 cos v 

k, = k,. 



ROTATION 



217 



From these equations it appears that 

Zj = cos cos <p cos ^ sin <p sin ^ 
m l = cos 6 cos (f> sin ^ + sin ^ cos ^ 
n! = sin cos v? 

Z 2 = cos 6 sin <p cos ^ cos <p sin ^ 
m 2 = cos 6 sin p sin ^ + cos p cos ^ 
n 2 = sin sin v? 

Z 3 = sin cos ^ 
w 3 = sin 6 sin ^ 
n 3 = cos 0. 

17. The Gyroscope. It is now possible to set forth in simplest 
terms the essential characteristics of the motion of a rotating 
rigid body, which is the basis of gyroscopic action. By a gyro- 
scope is meant a rigid body spinning at high velocity about an 
axis passing through the centre of gravity, which is at rest, and 
acted on by a couple whose representative vector is perpendicular 
to the axis. 

Consider, in particular, the following motion. Let A = J?, 
C 7* 0, and let the axis of f be caused to rotate with constant 
angular velocity, c, in the plane ^ = 0. What will be the couple? 
Here, d\l//dt = and Euler's Geometrical Equations give 



P 



dO 



de 

3~T7* T = 



where dd/dt = c. The components L and M are unknown, 
but N = 0. The third of the Dynamical Equations becomes : 



~ 
dt 



= 0; hence r = v, 



and P is a large positive constant. Since here 

d<p . 



Hence, from the first two equations, 

p = c sin vtj q = c cos vt. 



218 MECHANICS 

On substituting these values in the Dynamical Equations, we 

find: 

L = Ccv cos vt, M = Ccv sin vt. 

We may think of the couple as made up of a force F acting 
at the point C : (, 77, f) = (0, 0, 1) in Fig. 105, and an equal and 
opposite force at 0. Then F will be tangent to the sphere at 
C. Let it be resolved into two components, one perpendicular 
to the (, f )-plane ; the other, in that plane. The first will have 
the value L, taken positive in the sense of the negative ry-axis ; 
the second will equal M, taken positive in the sense of the -axis. 
When t = 0, 

L = Ccv, M = 0, 

and at any later time, the result is the same. This can be seen 
directly from the nature of the problem, since the motion of the 
axis of f in the plane \f/ = is uniform, and hence the force which 
the constraint exerts will be the same force relative to the body 
at one instant as at any other instant. 

It is easy to verify analytically the truth of the last statement. 
For, the force normal to the plane \l/ = will always be 

L cos <p M sin <p = Ccv ; 
and the force in that plane will always be 

L sin if> + M cos p = 0. 

This result brings out in the simplest form imaginable the 
essential phenomenon in gyroscopic action, namely, this: To 
cause the axis to move in a plane with constant angular velocity, 
a couple must be applied whose forces act on the axis in a direction 
at right angles to that plane. 

Finally observe that if one thinks of onesolf as 
standing on the gyroscope and moving with it, one's 
e exerted body along the positive axis of f and facing in the 
direction of the motion of the axis, the force L ap- 
plied to the gyroscope will be directed toward one's 
left, and hence the reaction of the gyroscope on the 
FIG. 107 constraint will be directed toward the right, the gyro- 
scope spinning in the clockwise sense as ono looks 
down on it. Of course, if the sense of the rotation were reversed, 
the sense of the reaction would be reversed also. 



ROTATION 219 

EXERCISES 

1. Show that, if no assumption regarding 6 is made, but ^ = 
and r = v, then 

T A - 4 d * e . n 4 de 

L = A sin vt -rz + Cv cos vt -T: 

at* at 

TM A * d * e n < dd 

M = A COS vt -T7T ~ Cv Sin vt -rr- 

at 1 at 

2. If the axis presses against a rough plane, \l/ = 0, the tan- 
gential force being p, times the normal force, then * 

dB 



provided dO/dt > and furthermore the point of the axis in 
contact with the plane moves backward, i.e. in the sense of the 
decreasing 6. 

On the other hand, the axis must have a sufficiently large 
radius so that the requirement below relating to the motion of 
the point of contact can be fulfilled. Hence 

dO c ^ t , Q cA ^ t 

37 = ce A and 9 = -/ Y e A 

at CIJLV 

whore c denotes the initial value of dO/dt, and initially = cA/Cp,v. 
Moreover, 

O 

VSS -T 8 ' 

where v = dO/dt and s = refer to the point in which the sphere 
(of radius 1) is cut by the axis. 

3. Prove that, in the problem of the preceding question, the 
normal reaction of the constraint is 



4. Show that, if a (small) constant couple, of moment , acts 
on the gyroscope, the vector that represents the couple being 
at right angles to the plane \l/ = and directed in the proper 

* If we think of the material axis as a cylinder of small radius, there will be a 
small couple about the axis, tending to reduce r. But as this couple approaches 
when the radius of the cylinder approaches 0, we may consider the ideal case of an 
axis that is a material wire of nil cross section, the couple now vanishing. 



220 MECHANICS 

sense, and if the axis of the gyroscope be constrained to move 
in the plane \l/ = 0, the acceleration of 6 is constant : 



This last equation is true, even when e varies with the time. 

6. Prove that, no matter how 8 varies, the axis of the gyro- 
scope always being constrained to move in the plane ^ = 0, 
the reaction on the constraining plane \l/ = is numerically 



its sense being that of the increasing \l/ when dO/dt > 0, but the 
opposite when dd/dt < 0. 

6. It has been shown that a rigid body is equivalent dynami- 
cally to three pairs of particles situated at the six extremities of 
a three dimensional cross ; 9. 

Let the equivalent system move as the gyroscope did in the 
text, i.e. with \l/ = and dO/dt = c. Consider, in particular, 
an instant, at which the moving axes are flashing through the 
fixed axes ; i.e. = <p \l/ 0. Show, by aid of the expres- 
sions for a, 0, 7, that the vector acceleration of each of the four 
particles on the - and the f-axes passes through ; but, in the 
case of each of the other two particles, is parallel to the axis of 
f . Hence explain the reaction of the gyroscope on the constraint. 

7. Discuss the problem of Question 2 for the case that the 
point of contact is allowed to slip forward. Consider also all 
cases in which dB/dt < initially. 

18. The Top. The top is a rigid body having an axis of 
material symmetry and, in the case of a fixed peg, supported at 
a point of the axis. Let the positive axis of f pass through the 
centre of gravity, (7, distant h from 0. 

The third of Euler's Dynamical Equations becomes, since the 
applied forces gravity and the reaction of the peg both pass 
through the axis of f , 

(1) C% = 0. 
Hence r = v (constant). 

The equation of energy here becomes : 

(2) A (p 2 + 2 ) + CV> = H - 2Mgh cos 6. 



ROTATION 



221 



Furthermore, the vertical component of the vector a is constant. 
For, the applied forces giving a vector moment at reduce to 
gravity, which is vertical, and so its vector moment with respect 
to O is horizontal. Now, the components of o- along the moving 
axes are Ap, Bq, and Cr. Hence the vertical component of a 

is ( 16) : 

Bqn 2 



On substituting for n lt n 2 , n z their values from 16 we have : 
(3) Ap sin 6 cos <p + Aq sin 6 sin <p + Cv cos = K. 
Turning now to Euler's Geometrical Equations, we find : 



(4) 



dt , - dO 
p = sin cos <p-~ + sin <p-jr 



... 
q = sin sin <p 



cos 



dO 
-=r 
at 



On substituting these values of p and q in (2) and (3) we find : 



(5) 



(6) 



sin 2 e -- = - bi> cos 



6 = 



C 



the constants a and depending on the initial conditions of the 
motion; i.e. they are constants of integration; whereas a and 
b are constants of the body. 

The third Equation (4) determines <p after and ^ have been 
found from (5) as functions of t : 



(7) 



<p = vt I cos 6 



dt 



dt. 



Returning now to Equations (5) and eliminating d\l//dt, we 
obtain : 

(8) sin 2 6 (~) 2 = sin 2 e(a - a cos 6) - (J8 - 6i> cos 0) 2 . 



222 MECHANICS 

The result is a differential equation for the single dependent vari- 
able, 6. It can be improved in form by the substitution 

(9) u = cos 9 : 

(10) 2 = (1 - u*)(a - au) - CJ - bvuY = f(u). 



Thus f(u) is seen to be a cubic polynomial, which we will 
presently discuss in detail. But first observe that the second 
Equation (5) gives : 

d * P "" bvu 



Hence \f/ is given by a quadrature after u has once been found 
as a function of t. 

Retrospect and Prospect. To sum up, then, we have reduced 
the problem to the solution of Equation (10) for u as a function 
of t.' Equation (9) gives 0; Equation (11) gives \f/; and Equa- 
tion (7) gives <p. We may concentrate, then, on the solution of 
Equation (10). 

19. Continuation. Discussion of the Motion. The Polynomial 
(1) fM = (1 - u*)(a - au) - (0 - bmY 

becomes positively infinite for u = + oo. It is negative or 
for u =+ 1, 1. Hence in general the graph will be as indi- 
cated, or 

</(M), u, <u<u 2 ] 

fM = /(iO = o. 

Moreover, 1 < u^ < u 2 < 1, and 
f(u) has one root, u' > 1. The roots 
w^ u 2 will, therefore, be simple roots. 
The differential equation 

(a)'- 

comes under the class discussed in Appendix B. In particular, 

the solution is a function 

(3) u = <*>(0 

single-valued and continuous for all values of t and having the 
period T 7 , where 




ROTATION 



223 




(4) 



or 

(5) <p(t + 
Furthermore, if 

(6) *! = 
then 

And similarly, if 

//w\ /, \ 

then 

/*7'\ /* \ /j I \ 

\t ) ^C*2 T ) ~ ^(^2 ~T~ Ty. 

Physical Interpretation. Let a sphere /S be placed about 
as centre, and let P be the point of intersection of the positive 
axis of f with S. Lot C be the curve that P describes on S. The 
results just obtained show that C lies between the two parallels 
of latitude corresponding to 

(8) u = u lt u = u 2 . 

For convenience let t be measured from a point on the upper 
parallel, u = u 2 . Then there are three cases according as initially 



III. < 0. 






CASE I. Since 



FIG. 109 



bvu 



eft 1 - u 2 

is positive when u has its greatest value, u 2j d^/dt will remain 
positive, and so ^ will steadily increase with t. Let ^ = when 
t = 0. As t increases to iT, \!/ will increase to 



224 MECHANICS 



where u = ^(0, Equation (3). When t = T, \p will have in- 
creased by ^, and one complete arch of the curve C will have 
been described. The arch is symmetric in the plane ^ = -J-^. 
The rest of C is obtained by rotating this arch about the polar 
axis of S through angles that are multipla of ^. 

CASE II. Here, d\f//dt is at the start, and hence 
|8 - bvu 2 = 0. 

Since u decreases, it follows that in the further course of the 
motion 

< bvu, 

and so \[/ steadily increases. The curve C has cusps on the upper 
parallel of latitude. 

CASE III. Here 

- bvu < 

at the start, and it is conceivable that this relation should persist 
forever. But even if this were not the case, it is still conceivable 
that the value of \l/ when P reaches the lower parallel of latitude 
should be less than or equal to the initial value, ^ = 0. That 
neither of these cases is possible that the value of \l/ corre- 
sponding to the first return of P to the upper circle is positive 
has been shown by Haclarnard.* The curve C has double points 
in this case, but it proceeds with increasing t in the sense of the 
advancing ^, as indicated. 

Special Cases. There is still a variety of special cases to be 
discussed, one of which is that in which f(u) has equal roots 
lying within the interval : 

1 < MI = tig < 1. 
Since 

/(I) 
in all cases, and since 



there must be a third root u 1 ^ 1. Thus u is a double root and 
f(u) = (w - u, 



where 

x(u) < 0, - 1 < u < 1. 

* Butt, des Sci. math. 1895, p. 228. 



ROTATION 225 

The only solution of Equation (2) in this case, which takes 
on the value u^ when t = 0, is 

u = w t . 

The curve C reduces to a parallel of latitude. 

When u = 1 is a root, various cases can arise. The point P 
may pass through the north pole with a velocity ; or it may 
gradually climb, approaching the north pole as a limit; or the 
top may permanently rotate about the polar axis. Similarly, 
when u = 1 is a root. 

There is a great wealth of literature on the gyroscope and 
the top. The reader can refer to the article on the Gyroscope 
in the Encyclopaedia Britannica; to Webster, Dynamics; to 
Routh, Elementary Rigid Dynamics; and to Appell, Mecanique 
rationelle, vol. II. 

EXERCISE 

Treat the case of a top on a smooth table. Assume that the 
peg is a surface of revolution. The distance, then, from the 
centre of gravity to the vertical through the point of contact 
with the table will be a function of the angle of inclination of 
the axis. 

Assume axes fixed in the body with the origin at the centre 
of gravity. 

Write down i) the equation of energy; ii) the equation that 
says that the vertical component of or is constant. 

From this point on the procedure is precisely as before, and 
the result is again a differential equation of the type treated in 
Appendix B. Discuss all cases, and show that in general the 
axis oscillates between two inclinations, both oblique to the 
vertical. 

Begin with the special case that the peg is a point. Having 
studied this case in detail, proceed to the general case and study 
it in detail, also. Then derive the special case as a particular 
case under the general case. 

20. Intrinsic Treatment of the Gyroscope.* The most general 
case of motion of a gyroscope reduces to one in which a single 
couple acts on the body, and this couple can be broken up into 

*The results of this paragraph arc contained in a paper by the Author: "On 
the Gyroscope," Trans. Amer. Math. Soc., vol. 23, April, 1922, p. 240. 



226 MECHANICS 

two couples one, represented by a vector at right angles to 
the axis of the gyroscope ; the other, by a vector collinear with 
the axis. In the most important applications that arise in prac- 
tice, the latter couple vanishes. But in the general case, it gives 
rise to the third of the Dynamical Equations in the form : 



The former couple can be realized by a single force F per- 
pendicular to the axis and acting at the point P in which the 
positive f-axis cuts the unit sphere, the other force of the 
couple and the resultant force acting at 0.* 

Definition of the Bending, K. Let C be the curve described 
on the unit sphere by P, and let S be the cone which is the locus 
of the axis of the gyroscope, and of which C is the directrix. Con- 
sider the rate at which the tangent plane to S is turning when P 
describes C with unit velocity. This quantity shall be denoted 
as the bending of the cone and represented by the number K. 
It is also the rate at which the terminal point of a unit vector 
drawn from at right angles to the tangent plane traces out its 
path on the unit sphere. K shall be taken positive when an ob- 
server, walking along C, sees C to the left of the tangent plane, 
and negative, when C is to his right. 

It is easy to compute K. Let V be the angle from the parallel 
of latitude through P with the sense of the increasing ^ to the 
tangent to C with the sense of the increasing s. Then it appears 
form an infinitesimal treatment that 



__ . 

v ' ds ds 

Since 

tan V = , . . -, or V = tan" 1 



, . . -, -77-; -, 

d\f/ sin B $' sin 0' 

where accents denote differentiation with respect to s, and since 

ds 2 - d6* + dj* sin 2 0, or /2 + V* sin 2 = 1, 
it follows that 
(3) jc = WB" - 0' iH sin - (1 + /2 ) V cos 0. 

* The point O need not be the centre of gravity in the following treatment. 
It may be any point fixed in the axis of material symmetry. 



ROTATION 227 

From the definition it follows at once that the bending of a 
cone of revolution must be constant. To find its value, let the 
coordinates be so chosen that the equation of the cone is = a. 
Then the length of the arc of C is 

5 = ^ sin a and so \l/' sin a = 1. 
From (3) it now is seen that 
(4) K = cot oc. 

The cone lies to the right of the observer, as he travels along C. 
If he reverses his sense, the sign of K will be changed. But both 
cases are embraced in the single formula (4), the second corre- 
sponding to a cone whose angle is TT a, or 
again for which s is replaced by s. 

Conversely, if K is constant, C is a circular 
cone. For, the equation (3) can, by elimi- 
nating ^', 



U - A x 1 f 

be written in the form : 

ntt 



(5) K = 

the sign holding whenever ^' < 0. Hence 





If K is constant, set K = cot a. Then Equation (6) admits 
one solution, = a, or = 7r a; and, as is shown in the 
theory of differential equations, this is the only solution which, 
at a point s = s , takes on the value a, or TT a, and whose 
derivative vanishes there. 
Further Formulas for K.* From (3) it follows further that 



-7-77: sin B 2 -J-T^ cos 6 sin 2 6 cos 



,~ , 

(7) * = 



where the sign holds whenever \f/' < 0. 

* These results are inserted for completeness. They will not be used in what 
follows, and the student may pass on without studying them. They are chiefly 
of interest to the student of Differential Geometry. 



228 



MECHANICS 



If K is known, or given, as a function of s, then Equation (6) 
determines as a function of s, and \l/ is then found by a quad- 
rature : 

(8) 

The bending, K, is connected with the curvature, K, of C, re- 
garded as a space curve, by the formula 

(9) K* = K 2 + 1. 
Furthermore, cf. Fig. Ill below: 

( i j k 

(10) n = a X t 



x y z 
x' y' z' 



(11) 
hence 

(12) 

Since I K\ = 1 1' I and 



= yz" - 



zx" - xz" 

KZ ' = xy _ y X ". 



(13) ^ 2 = x"* + y"* + z"*, 

formula (9) follows at once from (12) and (13). Moreover, from 
(12) it follows that 



(14) 



*=- 



x y z 
x' y' z' 
x" y" z" 



Finally, the torsion, T, of C is connected with /c by the relation : 

v l *= T, 
the result obtained by Professor Haskins.* 

* For the proof of this formula cf. the Author's paper cited above. 



d 
Ts ( 



ROTATION 229 

21. The Relations Connecting v, F, and *. The physical phe- 
nomenon which it is most important to bring home to one's 
intuition is the effect of the force F on the motion of the gyro- 
scope. Any such explanation must take account of all three 
quantities, v, F, and K. But many popular explanations claim- 
ing correctly to be "non-mathematical," but incorrectly to be 
accurate in their mechanics fail because they are unaware 
of K. Thus, for example, the statement often made that " when 
a couple is applied to a rotating gyroscope, the forces of the 
couple intersecting the axis of the gyroscope at right angles, the 
axis will move in a plane perpendicular to the plane of the forces 
of the couple" is false. In fact, the axis will begin to move 
tangentially to this plane, if it starts from rest, and all inter- 
mediate cases are possible, according to the initial motion of the 
axis. 

A simple and accurate explanation, in terms of v, F, and K, 
can be given as follows.* First of all, however, the third of 
Euler's Dynamical Equations, which here becomes : 



(1) 



and requires no further comment than i) that it is perfectly 
general, applying to the motion of the gyroscope under any 
forces whatever; and ii) that in the case which most interests 
us, namely that in which there is only the force F (and the reac- 
tion at 0) we have : N = 0, and so r = *>, a constant. 

Let F, then, be resolved, in the tangent plane, into a component 
T along the positive tangent, and a component Q, taken positive 
when directed toward the left of the observer; i.e. Q is posi- 
tive when K is positive. Then 



(2) 



AKV* + Crv = Q, 



where v = ds/dt and s increases in the sense of the motion of P, 
r being given by Equation (1). 

*Cf. the Author's paper "On the Gyroscope" cited above, p. 240. 



230 



MECHANICS 



Proof. Let the unit vector from to P be denoted by a (it 
is the vector 7 of the coordinate system) ; let t be a unit vector 
along the positive tangent to C at P; and let n be a unit 

vector normal to a and t and so oriented 
' a with regard to them as ft is with regard 

\p X to 7 and a. These are principal axes of 

t \ inertia, and the moments of inertia about 

them are : 

L = A I n = A, I a = C. 




The components of the angular velocity 
& about them are : 



FIG. Ill 



o>t = 0, w n = I), 
Now, (T has the value : 

a = I n C0 n n + It CO* t + I a C0 a a. 

Hence 

(3) 



From this equation we can compute -rr : 



do- 



dv 



dn 



da 



It is clear that 
(4) 



da 
dt 



vt. 



Furthermore, from the definition of the bending, it appears that 
/^x dn 

(5) -j-r = KVt 

Hence, finally, 
d<r 



(6) 



= Av-n + (Aw* + C)t + C 



Let the vector M which represents the resultant moment of 
all the applied forces about be written in the form : 

M = M n n + M t t + M a a. 
Since 

da -. 



ROTATION 231 

we have : 

(7) Av^- = M n , A K v* + Crv = M t , C % = M a . 
us dt 

Turning now to the case in which we are most interested, 
namely, that in which a force F acts at P in a direction at right 

angles to OP : 

F=-Qn+Tt, 

we see that M n = T, M t = Q, and thus Equations (2) are 
established. Equation (1) is the third of Equations (7). 

We have thus obtained Euler's Dynamical Equations in the 

form: 

dv 



(8) 



Av^- = T 
ds 

AKV* + Crv = Q 



22. Discussion of the Intrinsic Equations. The first of Equa- 
tions (8), 21, 

AV = r, 

ds ' 

admits a simple interpretation. It shows that the point P de- 
scribes the curve C exactly as a smooth bead of mass m = A 
would move along a wire in the form of C if it were acted on by 
a tangential force T. 
The third equation, 

C~ = N 
^ dt *' 

shows that the component r of the angular velocity & about the 
axis of the gyroscope varies exactly as it would if the axis were 
permanently at rest and the same couple N relative to the axis 
acted. 

The second equation, 
A) AKV* + Crv = Q, 

expresses the sole relation which holds between the four variables 

K, v, r, and Q. In the applications, however, r is constant, r = v, 

and so the equation 

A') AKV* + Cw = Q 

expresses the sole relation between K, v, and Q. 



232 MECHANICS 

The Case F = 0. Let us begin with the case that F vanishes, 
but the axis is not at rest. Here, Q = 0, T = 0. Equation A) 
gives 

i) AKV + Cr = 0, 

or, on introducing the radius of bending, p = 1/| K |, and choos- 
ing r > : 

Av 
p== 'Cr' 

If r is a positive constant, r = v > 0, then 

Cv 



and since v is constant, for 




A __ n 
FIG. 112 ds~ ' 

K is also constant, and negative. The axis of the gyroscope is 
describing a cone of semi-vertical angle a, where 

cot a = | K |, or tan a = p, 

and the sense of the description is such 
that the observer, walking along C in the 
positive sense, has the cone on his right. 

The Case K = 0. Here, the path of P 

is an arc of a great circle, and 

& ' FIG. 113 

Q = Crv, or Q = Cw, 

no matter what T and the motion of P along its path may be. 
The pressure of the axis against the constraint, in a normal direc- 
tion, is to the right, and is proportional to r and to v ; or, if 
r is constant, to v, the coefficient then being Cv. Thus we obtain 
anew, and with the minimum of effort, the main result of 17. 

General Interpretation of Equation A). We can now give a 
simple physical interpretation to Equation A) : 

Am* + Crv = Q. 

The left-hand side is the sum of two terms. The second term 
expresses the force, 

Q 2 = Crv, 



ROTATION 



233 



that would be required to cause P to describe a great circle on 
the sphere; i.e. to make the axis move in the plane through 
tangent to C. This force, Q 2 , is always directed toward the 
left, for Q 2 > 0. 
The first term, 



accounts for the bending. 



~ , 9 

Q l = AKV*, 

Its numerical value, 



can be interpreted as the centripetal force exerted on a particle, 
of mass m = A, to make it describe a circle of radius p with 
velocity v. Wlien K is positive, this force is positive, and so is 
directed toward the left ; and vice versa. 

Consider now the force Q f along the normal n at P, which 
(combined with the smooth constraint of the surface of the sphere) 
would be required to hold a particle of mass m = A in the path C. 
Let the vector a be written in the form : 



Then 



a = xi 



yj + zk. 



v = xi + y] + zk = vt, 
where x' = dx/ds t x = dx/dt, etc. Furthermore, 

n = a X t = (yz f - zy f ) i + (zz' - xz f ) j + (**/' - yx')k. 
The acceleration, (a), of P in space is, of course : 

() = zi + j + ^k. 

Now, the component of the acceleration along the normal n 
to the plane of a and t is n-(a), which can be written in the 

form : 

x y z 

x' y f z' 

x y z 
Since x = vx', it follows that 

x = v*x" + vx', etc., 
and so 



x y z 
x' y' z' 
x y z 



x y 



x" y" z" 




234 MECHANICS 

Thus mw 2 is equal to the force Q' tangent to the sphere and 
normal to (7, which would be required to hold a particle of mass 
w, describing (7, in its path; the component along t being 
mvdv/ds, and the third component, along a, being the reaction 
normal to the sphere, in which we are not interested. 

It is natural to think of the point pn on the line through P 
along n as the centre of bending. If we draw the osculating cone 
of revolution through P, this is the point Q in which 
that line meets the axis of the cone. An obvious 
interpretation for this force of mw 2 is the centripetal 
force of a particle describing a circle of radius p, with 
centre at Q, tangent to C at P, the velocity being v. 
_, . The force Q 2 can be realized physically as follows. 
Let an electro-magnetic field of force be generated by 
a north-pole situated at 0, and let the particle m carry a charge, 
e, of electricity. The force exerted on e by the field will be at 
right angles to the path and tangent to the sphere, and, 
finally, proportional to the velocity, v, of m. Hence e can be so 
chosen that this force will be precisely equal to Q 2 = CW. 

In the more general, but less interesting, case that r is variable, 
the physical interpretation can still be adapted by using a variable 
charge.* 

Summary of the Results. To sum up, then, we can say : The 
point P, in which the axis of the gyroscope meets the unit sphere 
about 0, moves like a particle of mass m = A constrained to 
lie on the sphere and carrying a charge of electricity, e. The 
forces that act on m are supplied by the electromagnetic force 
of the field, Q 2 = Cw, acting on e y and a force F acting on m, 
the components of F along the tangent and normal at P being 
T and Q l respectively. The case of a variable r can be met by 
a variable charge, e. 

As regards the physical realization of the condition that the 
particle lie on the surface of the sphere, we may think of a mass- 
less rod of unit length, free to turn about one end which is pivoted 
at 0, and carrying the particle at the other end. 

* The idea of using the above electro-magnetic field to obtain #2 was suggested 
to me by my colleague, Professor Kemble, to whom I had just communicated the 
results of the text, down to this point. (Note of Jan. 23, 1933.) 



ROTATION 235 

EXERCISES 

1. Suppose the axle P of the gyroscope is caused to move in 
a smooth slot in the form of a meridian circle, which is made to 
rotate in any manner. The force F will then be normal to the 
meridian, or tangent to the parallel of latitude. Show that 

d 2 6 . 



Suggestion : Combine Euler's Geometrical Equations with 
Euler's Dynamical Equations. 

2. Let the components of F along the meridian in the sense 
of the increasing 6 and along the parallel of latitude in the sense 
of the increasing ^ be denoted respectively by and ^ Show 
that 



If and ^ are known as functions of 6, \f/ } t, these equations 
suffice to determine the path of P. 

3. Consider small oscillations of the axis of the gyroscope in 
the neighborhood of the axis 6 = v/2, $ = 0. Let 



Show that the equations of Question 1 lead to the approximate 
equations : 



4. Generalize the equations of Question 2 to the case that A, 
, C are all distinct. 



236 MECHANICS 

5. Intrinsic Equations. From the equations : 

Av% = T, 

ds ' 

AKV* + Cvv = Q, 



K = 




the path can be determined if T, Q are known as functions of 
s and v. 

6. . Ship's Stabilizer. The gyroscope can be used to reduce the 
rolling of a ship. A massive gyroscope is mounted in a cage, 
or frame, its axis being fixed with reference to the frame, and 
vertical. The frame is mounted on trunnions, with axis hori- 
zontal and at right angles to the keel, and it is provided with 
a brake to dampen its oscillations about this axis. Thus the 
axis of the gyroscope has two degrees of freedom; it can rotate 
in the plane through the keel and the masts, and this plane rotates 
with the rolling of the ship.* Isolate the following systems : 

i) The ship, exclusive of the gyroscope and frame ; 
ii) The frame ; 
Hi) The gyroscope. 
The rolling of the ship is governed by the equation : 



where the first term on the right is due to the damping of the 
water; the second, to the righting moment produced by the 
buoyancy ; and the third, to the force exerted by the trunnions. 

The frame may be thought of as rotating about the point, 0, 
regarded as fixed, in which the axis of the gyroscope cuts the 

*A picture and an account of the ship's gyroscope is found in the article on 
the "Gyroscope" in the Encyclopaedia Britannica and in Klein-Sommerfeld, 
Theorie des Kreisels, vol. iv., p. 797. For the discussion which follows the reader 
also needs, however, the theory and practice of Oscillatory Motion with Damping ; 
cf. the Author's Advanced Calculus, Chap. XV. 



ROTATION 237 

axis of the trunnions. Let Euler's Angles be so chosen that the 
axis of the sphere : 6 = 0, ^ = 0, is parallel to the keel, the 
plane ^ = being vertical. Moreover, let be replaced by $, 
where 



The motion of the gyroscope about its centre of gravity, the 
point (9, will be governed by the approximate equations of Ques- 
tion 3. 

Finally, the motion of the frame is governed by the equations 
called for in Question 4 above. These equations are modified by 
the condition <p = 0, and then reduced still further by setting 
sin & = 0, cos # = 1. Thus 



dt 



where the first term on the right is due to the brake and other 
damping, and the second, to gravity, since the frame is so con- 
structed that its centre of gravity is appreciably below O. 

On combining these five equations and neglecting. A + A' in 
comparison with 7 we find : 



These are the equations which govern the motion. They are 
discussed at length in Klein-Sommerfcld, I.e. 

23. Billiard Ball. Let a billiard ball be projected along the 
table, with an arbitrary initial velocity of the centre, 0, and an 
arbitrary initial velocity of rotation. To determine the motion. 

Let the (x, y)-plane of the axes fixed in space be horizontal. 
Let moving axes of (, 17, f) be chosen parallel to (#, y, z), but 
with the origin at the centre of the ball. 

The point of the ball P, in contact with the table, shall be 
slipping, and the angle from the positive direction of the axis 
of x or to the direction of its motion shall be ^. 



238 



MECHANICS 



The forces acting are : gravity, or M g t downward at R = M g 
upward at P ; and the force of friction, nMg, at P in the sense 
opposite to that of slipping. Hence, for the motion of the centre 
of gravity, 

M -jp = pM g cos \f/ 

CD rf2 . 

dt 2 

The vector momentum a-, referred to the centre of gravity, 
has for its components along the moving axes : 



where 

The moment equation, 

thus gives : 



f Ma 2 . 



d<r 



(2) 



Hence 
(3) 



/ - = nMga sin 

u-6 

7 -- = nMga cos ^ 



'if- - 



= const. 



5 dt 



The angle ^ is unknown. Eliminate it by combining Equa- 
tions (1) and (2) : 



(4) 

Hence 

(5) 



dt* 

^y. 

dt 2 



5 dt 
2a 



2a 



where A, B are constants of integration depending on the initial 
conditions. They may have any values whatever. 



ROTATION 239 

Let V be the velocity of the lowest point of the ball. Then 



(6) 



V x = V cos $ = -7- aco, 
V v = V sin ^ = - + au(. 



Combining these equations with (5) we get : 



where 



2\dt ^ 

A' = - 



B' =- fB. 



Equations (1) now take on the following form. For abbrevi- 
ation let 



dt 



A', 



Then 

(8) 

Hence 

and consequently 



du 
dt 

dv 



du dv ^ 

v -7T u -77 = 0, 

dt dt y 



av, 



where a, /3 are constants not both 0. Moreover, u and v are 
not both 0. 

Suppose u > 0, a > 0. Then 



av 



av 



u 



The proof of this last equation requires the consideration of the 
two cases : i) 7* ; ii) = 0. These formulas are general, 
holding in all cases in which w ^ 0. 



240 



MECHANICS 



It thus appears that 



(9) 



cos 



sn = 



ft 



Hence d?x/dt 2 and d 2 y/dt* are constants, and consequently the 
centre of the ball describes in general a parabola; in particular, 
a straight line. The direction, however, in which the point P 
is slipping, is always the same; cf. Equations (9). 

This result comprises the main interest of the problem, so long 
as there is slipping. Slipping ceases when V = 0, or 



(10) 



The Subsequent Motion. From this instant on the motion is 
pure rolling we are, of course, neglecting rolling friction and 
all other damping. For, at the instant in question, V 0, and 
the angular velocity is related to the linear velocity of the centre 
of gravity as follows. Let the centre of the ball be at the origin 
and let its velocity be directed along the positive axis of x. Then 



(11) 



dx 
Tt 



t-O 



c # 
c > Jt 



0; 



au( | t-o = 0, aco, \ t -o = c, wf | t-o y, 

where 7 can have any value, positive, negative, or 0. 

Let us consider the motion which consists in pure rolling and 
pivoting, and see what force at P is necessary. First, we have 



(12) 



M w = 



- 
dt* 



- Y 
~ Y> 



where X, Y are the components of the unknown reaction at P. 
Next, taking moments about the centre of gravity, we find : 



(13) 



UOi) f UWf) -w* 

___. i ___. _ ax 
dt dt 



dt dt 



ROTATION 241 

Finally, 



(14) 



Tr A 

y. - - - a*, - 



These seven equations, (12), (13), (14), together with the 
initial conditions (11), formulate the problem completely, and 
determine the seven unknown functions, x, y, co$, w^, o^, X , F, 
as we will now show. 

From the second equation (13) it appears that 



Subtracting this equation from the first equation (12), we find : 



But the left-hand side of this equation vanishes because the first 
equation (14) is an identity in t. Hence X = 0. Similar con- 
siderations show that Y = 0. 

On substituting these values in (12) and (13), these five equa- 
tions can be solved subject to the five initial conditions (11), and 
the other condition, that initially x = 0, y = 0. The centre of 
the ball describes the positive axis of x with constant velocity, c. 
The angular velocity w is also constant, its components along 
the axes being given by their initial values (11). Since 7 is 
arbitrary, w may be any vector whatever in the (77, f)-plane, 
whose component along the r;-axis is c/a. 

The foregoing discussion may be abbreviated by means of the 
Principle of Work and Energy, Chapter VII. 

The motion of pure rolling with pivoting requires, then, no 
force to be exerted by the table. It is uniquely determined by 
the initial conditions, and hence it coincides with the actual 
motion of the billiard ball. 

24. Cart Wheels. Consider the forewheels of a cart. Ideal- 
ized they form two equal discs connected by an axle about which 
each can turn freely. To determine the motion on a rough 
inclined Diane. 



242 



MECHANICS 



We will begin with a still simpler case that of a single wheel, 
or disc, mounted so that it can turn and roll freely, but will always 
have its plane perpendicular to the plane on which it rolls. The 
frame which guides it may be thought of as smooth. Its mass 
can be taken into account, but we will disregard it, in order not 
to obscure the main points of the problem. 

We will choose the coordinates as indicated, the axis of being 
in the disc and always parallel to the plane ; the axis of 77, being 

the axis of the disc, is also 
parallel to the plane. The 
axis of y lies in the plane and 
is horizontal. The axis of x is 
directed down the plane. Let 
v? be the angle through which 
the disc has turned about the 
axis of rj ; let s be the arc de- 
scribed by the point of con- 
tact, P ; and let be the angle 

from the positive axis of x to the positive tangent at P. Let the re- 
action of the plane be 

F = Xa + Yj9 + Z T , 

where a, 0, y are unit vectors along the moving axes. 
Z = Mg cos e, where e is the inclination of the plane, and 




Then 



(1) 



d 2 x 
M -;- X cos 6 Y sin 6 + Mg sin 6 



= Xsin0 + Ycos0 



The angular velocity, 

has the value 

Moreover, 

= - da, 7 = 0. 

Take moments about the centre of gravity : 



(2) 



dt 



ROTATION 



243 



Since 

and A = C = 

Hence 

or 
(3) 



In computing the right-hand side of Equation (2), the couple 
which keeps the axis of the disc parallel to the plane must be 
taken into account. The vector which represents it is collinear 
with the axis of . Hence the couple may be realized by the two 
forces : 



= 0, co,, = <p, o> 
a 2 , # = pf a 2 , we have : 






= - Beta. + 5^j3 + 



Thus 



at r 2 =-0. 



r* X F* = j8 X F l7 + (- 18) X (- F,y) + (- ay) X F; 



r* X F, = (2F, + aY) a - aX0. 



or, finally : 
(4) 

Equating, then, the vectors (3) and (4) we find : 



(5) 



Finally, the condition of rolling without slipping can be written 
in the form : 



dx 
~dt 



= v cos 0, 



dy = 
dt 



v sin ^, 



244 MECHANICS 

where 



and so 

/n\ dx d<p n dy d<p . 

(6) -TT = a-- cos 0, -~ = a- sin 0. 
v ' dt dt dt dt 

The formulation is now complete. There are seven unknown 
functions, namely : x, y, 0, p, X, Y, F l9 and seven equations to 
determine them, namely, Equations (1), (5), (6). 

To solve these equations, begin by determining 6 from (5) : 

3/\ 

(7) f t = X, 9 = \t + M . 
Next, eliminate Y in (1) : 



cos<9 + sin ^ = x + Mg sin e cos 6. 
at 1 di L J 

And now X can be eliminated by (5), and x y y by (6). Thus 



Ma - = i Ma ~ + Mg sin e cos 0, 



or 

(8) 

where 



Hence 

(9) ^ = *(sin-slnM) + *o, 

and 

fc , M . / . fc sin M\ . 

v? = ^5 (cos M - cos 0) + ^ -- Jt + v?o- 

From (6), x and y can now be found as functions of t; and finally 
X, Y, F u can be determined from (1) and (5). 

The system of Equations (1), (5), (6) is an example of equa- 
tions called non-holonomic by Hertz because some of them, 
namely (6), involve time-derivatives of the first order only 
and cannot be replaced by geometric equations between the 
coordinates. 

An interesting case of a non-holonomic problem is that of a 
coin rolling on a rough table. It is studied in detail by Appell, 



ROTATION 245 

Mecanique raiionelle, Vol. I, p. 242, of the 1904 edition, and an 
explicit solution is obtained in terms of the hypergeometric 
function. 

EXERCISES 

The student should first, without reference to the book, repro- 
duce the treatment just given in the text, arranging in his mind 
the procedure: i) figure, forces, coordinates; ii) motion of the 
centre of gravity; Hi) moments about the centre of gravity; 
iv) conditions of constraint ; v) the solution of the equations. 

1. Solve the problem of the two wheels mentioned in the 
text. 

2. Coin rolling on a rough table. Read casually Appell, 
adopting his system of coordinates. Then construct independ- 
ently the solution, following the method used in the problem 
of the text. 

3. The problem of the text, when the mass of the frame is 
taken into account. Begin with the case that the bottom of the 
frame is smooth and its centre of mass is at the centre of the disc. 

4. Study the motion of the centre of gravity of the disc treated 
in the text, by means of the explicit solution of x, y in terms of t. 

25. Resume. In dealing with the motion of a rigid body, 
there are the two vector equations : 



equivalent to six ordinary equations. 

It is always possible to take moments about the centre of 
gravity. 

The Principle of Work and Energy frequently gives a useful 
integral of the equations of motion. 

If the right-hand side of the Moment Equation is a vector 
lying in a fixed plane, the component of a normal to this plane is 
constant, and thus an integral of the equations of motion is 
obtained. 

Sometimes there are conditions which are expressed by equa- 
tions between time-derivatives of the first order, t = t, but which 
cannot be expressed by equations between the coordinates only. 



246 MECHANICS 

The first step in solving a problem is to draw the figure, mark 
the forces, and pass in review each of the items just mentioned ; 
reflecting, in case these are not adequate, on considerations of 
like nature, which may be germane to the problem. 

With the forces and the geometry of the problem in mind, 
next choose a suitable 

Coordinate System. If it is desirable to refer a to the centre 
of gravity, a Cartesian system with its origin there is usually 
the solution. These axes may be fixed in the body, coinciding 
with the principal axes of inertia. Or their directions may be 
fixed in space. Or they may move in the body and in space 
subject to some condition peculiar to the problem in hand. 

Final Formulation. It remains to write down the equations 
arising from each of the above considerations. They must be 
in number equal to the number of unknown functions. Besides the 
differential equations of the second order, these may also include 
differential equations of the first order, not reducible to equations 
between the coordinates. 

The solution of these equations is a purely mathematical prob- 
lem. Go back frequently over familiar problems and recall the 
mathematical technique, writing the equations down on paper, 
neatly, and carrying through all details of the solution. In this 
way, analytical consciousness is developed; it is composed of 
experience and common sense. 

Further Study. There is a vast fund of interesting problems 
in Rigid Dynamics, of all orders of difficulty, and two invaluable 
treatises are Appell, Mecanique rationelle, Vols. I and II, and 
Routh, Rigid Dynamics, Vols. I, II. Routh's exposition of the 
theory is execrable, but his lists of problems, garnered from the 
old Cambridge Tripos Papers, are capital. 

The earth is a top, and the study of the precession and nuta- 
tion of the polar axis is a good subject for the student to take 
up next. 

Webster's Dynamics is also useful in the important applica- 
tions it contains. The text is hard reading; but the student 
who once dominates the method as set forth, for example, in the 
foregoing treatment, can and should construct his own solution 
of the problem in hand. 

Finally, Klein-Sommerfeld, Theorie des Kreisels y in four volumes. 
This is a classic treatment of the subject. The first three vol- 



ROTATION 247 

umes treat the theory of the top by modern mathematical methods. 
The fourth volume, devoted to the applications in engineering, 
can be studied directly through the theory which we have de- 
veloped above, without reference to the earlier volumes. There 
is a detailed study of the gyroscopic effect in the case of rail- 
road wheels, the Whitehead torpedo, the ship's stabilizer, the 
stability of the bicycle, the gyro-compass, the turbine of Leval, 
and a large number of further topics. 



CHAPTER VII 
WORK AND ENERGY 

1. Work. In Elementary Physics work is defined as the 
product, force by distance : 

(1) W = Fl, 

the understanding being that a force F, constant in magnitude 
and direction, acts on a particle, P, or at a point P fixed in a 
rigid or elastic body, and displaces P a distance I in the direction 
of tho force. 

The definition shall now be extended to the case of a variable 
force, still acting on a particle or at a fixed point of a material 

body. Let 

a ^ x g 6 

be the interval of displacement. Let 

F=f(x) 

be the force, where f(x) is a continuous function. Divide the 
interval into n parts by the points X Q = a, x l9 , x n -\, x n = b, 
F k and consider the fc-th sub-interval : 



- _, . 

FlG 116 3*-i ^ x ^ x k , Az* = x k - _!. 

And now we demand that the extended definition of work shall 
be so laid down that 

i) the total work shall be equal to the sum of the partial works : 



ii) the work for any interval shall lie between the work cor- 
responding to the maximum value of the force in that interval, 
and the work corresponding to the minimum force : 

g AW k ^ 

248 



WORK AND ENERGY 249 

where 

Fi F Fi' 

in the interval in question. 

Now, since f(x) is a continuous function, it takes on its mini- 
mum value, Fi, in the interval : 



and similarly, its maximum value : 

FZ =/(*;'), **- 

Hence W lies between the two sums : 



But each of these sums approaches a limit as n increases, the 
longest Axjb approaching 0, and this limit is- the definite integral : 



Hm 



i> 

= f 
J 



Hence the requirements, i.e. physical postulates i) and ii) are 
sufficient to determine the definition of the work in this case : * 

b 

(2) W=Jf(x)dx. 

a 

The foregoing definition applies to a negative force, and also to 
the case that 6 < a ; the work now being considered as an alge- 
braic quantity. Thus if a force, instead of overcoming resistance, 
is itself overcome ; i.e. yields, it does negative work. 

The work which corresponds to a variable displacement, x, 
where a ^ x ^ 6, is by definition : 

X 

(3) W=Jf(x)dx. 

a 

Hence 

(O f - ,. 

* Strictly speaking, we have shown that (2) is a necessary condition for the 
definition of work according to the postulates i) and ii) . It is seen at once, however, 
that conversely Equation (2) affords a sufficient condition, also. 



250 MECHANICS 

EXERCISES 

1. Show that the work done in stretching an elastic string is 
proportional to the square of the stretching. 

2. Find the work done by the sun on a meteor which falls 
directly into it. 

3. The work corresponding to a variable displacement from 
x to 6, where a ^ x ^ 6, is by definition : 

& 

(5) W=ff(x)dx. 

X 

What is the value of dW/dxl 

2. Continuation : Curved Paths. Suppose the particle describes 
a curved path C in a plane, and that the force, F, varies in mag- 
nitude and direction in any continuous manner. What will be 
the work done in this case? 

Suppose the path C is a right line and the force, though oblique 
to the line, is constant in magnitude and direction; Fig. 117. 

Resolve the force into its 
two components along the line 
and normal to it. Surely, we 
tett >f < j*a must lay down our definition 

r^ - -~- i of work so that the work done 

\ii \ 

by F is equal to the sum of 




FlG 117 the works Of the component 

forces. Now, the work done 

by the component along the line has already been defined, namely, 
Fl cos ^, where F = | F | is the intensity of the force. 

It is an essential part of the idea of work that the force over- 
comes resistance through distance (or is overcome through dis- 
tance). Now, the normal component does neither; it merely 
sidles off and sidesteps the whole question. It is natural, there- 
fore, to define it as doing no work. Thus we arrive at our final 
definition: The work done by F in the particular case in hand 
shall be 

(6) W = Fl cos ^. 

A second form of the expression on the right is as follows. Let 
X and Y be the components of F along the axes. Let T be the 
angle that the path AB makes with the positive axis of x. Then 



WORK AND ENERGY 



251 



the projection of F on A B is equal to the sum of the projections 
of X and Y on AB, or 

F cos ^ = X cos T + Y sin T. 
On the other hand, 

x 2 x l = I cos T, 2/ 2 2/i = Z sin r. 
Hence 

(7) TF = X(x z arO H 



General Case. If C be any regular curve, divide it into 
n arcs by the points s = 0, s t , , s n -i, s n = J. Let F be 
the value of F at an arbitrary point of 
the /b-th arc, and let ^i be the angle 
from the chord (s t -i, s k ) to the vector 
F. Then the sum 



Jb-l 




FIG. 118 



where Z fc denotes the length of the 
chord, gives us approximately what we should wish to understand 
by the work, in view of our physical feeling for this quantity. 
The limit of this sum, when the longest h approaches 0, shall be 
defined as the work, or 



(8) 



W 



Since 



~^- = 1, 

As* ' 



it is clear that the above limit is the same as * 

/ 

n /* 

lim V Fk cos fa Asfc IF cos \l/ ds. 

A J 

We are thus led to the following definition of work in the case 
of a curved path : 

iF cos ^ ds. 

o 



(9) 



W 



* Cf. the author's Advanced Calculus, p. 217. It is imperative that the student 
learn thoroughly what is meant by a line integral. 



252 MECHANICS 

A second formula for the work is obtained by means of (7) : 
< i 

(10) W= Ax COST + 7 SUITES = C(x^ + Y- 

J J ^ as t 



or 

(11) W = Cxdx + Ydy. 

The extension to three dimensions is immediate. The defini- 
tion (9) applies at once without even a formal change. Formula 

(11) is replaced by the following : 

(12) W = Cxdx + Ydy + Zdz 
or 

(', 6'. c') 

Cxdx+Ydy + Zdz. 

(a.b.c) 

Example. To find the work done by gravity on a particle 
of mass m which moves from an initial point (X Q , y Q , Z Q ) to a final 
point (x lt y lt zj along an arbitrary twisted curve, C. 

Let the axis of z be vertical and positive downwards. Then 

X = 0, Y = 0, Z = mg ; 
W = jXdx + Ydy + Zdz = jmgdz = mg(z l - z ). 

C ZQ 

Hence the work done is equal to the product of the force by the 
difference in level (taken algebraically), and depends only on 
the initial and final points, but not on the path joining them. 

EXERCISES 

1. A well is pumped out by a force pump which delivers the 
water at the mouth of a pipe which is fixed. Show that the 
work done is equal to the weight of the water initially in the well, 
multiplied by the vertical distance of the centre of gravity be- 
low the mouth of the pipe. 

2. The components of the force which acts or? a particle are : 
X = 2x 3y + 4z 5, Y = z x + 8, Z = x + y + z + l2. 



WORK AND ENERGY 253 

Find the work done when the particle describes the arc of the 

helix 

x = cos 0, y = sin 0, z = 70, 

for which ^ g 2*. 

3. If the curve C is represented parametrically : 
C: x= /(X), y = *(X), = f (X), X S X ^ Xi, 
show that the work is given by the integral : 



3. Field of Force. Force Function. Potential. A particle 
in the neighborhood of the solar system is attracted by all the 
other particles of the system with a force F that varies in magni- 
tude and direction from point to point. Thus F is a vector point- 
function throughout the region of space just mentioned. Its 
components along Cartesian axes, namely, X, Y y Z, are ordinary 
functions of the space coordinates, x, y, z, of the particle. In 
vector form : 
(1) F = Xi + Y j + Zk. 

The example serves to illustrate the general idea of a field 
of force. We may have an electro-magnetic field, as when a 
straight wire carries a current. If the north pole, P, of a magnet 
is brought into the neighborhood of the wire, it will be acted on 
by a force F at right angles to any line drawn from P to the wire 
and of intensity inversely proportional to the distance of P from 
the wire, the sense of the force depending on the sense of the 
current. 

If the axis of z be taken along the wire, then 

Z-0, 



where (r, 0, z) are the cylindrical coordinates of P, and C is a 
positive or negative constant. Thus in vector form 



and 



254 MECHANICS 

Force Function. It may happen that there is a function 

(4) u = <p(x, y,z) 

such that 

, v Y _ du v _ du 7 __ du 

(5) X ~te> W ~d~z 

Such a function, w, is called a force function. In vector form : 



F can be written in symbolic vector form as follows. Let 
V be a symbolic vector operator, namely : 

(7) V = i +' + k - 

Then Vu is defined as : 

Hence 

(9) F = Vu. 

Gravitational Field. In the case of the field generated by a 
single particle of attracting matter, there is a force function : 

(10) = 

where r is the distance from the given fixed particle to the variable 
particle, and X is a positive constant. 
In the case of n particles, 

(n) - 2 T k > 

provided the units are properly chosen. 

Ekctro-Magnetic Field. For the electro-magnetic field above 
described, 

(12) 11 = CO. 
We may also write : 

(13) u = C tan~ l -; 

v / X 9 

but this formula is treacherous, since only certain values of the 
multiple-valued function are admissible. However, since the 
wrong values differ from the right ones only by additive con- 



WORK AND ENERGY 255 

stants, we can use the formula for purposes of differentiation, 
and we shall have : 

(14) X = |H = C-=g- v Y = f* - C^jhi, Z = 0. 
' dx x 2 + 2/ 2 ' ?/ x 2 + y 2 

Work. When a particle describes an arbitrary path in a field 
of force, the work done on the particle by the field is given by 
Equation (12) of 2. If there is a force function, this formula 
becomes : 

i i &u 7 . du , \ 



i.e. the change which u experiences along the curve C. If the 
region in which C lies is simply connected, or if u is a single- 
valued function, then 

(16) W = u + const. 

Thus W is independent of the path by which the particle arrived 
at its final destination, and depends only on the starting point 
and the terminal point : 

(17) W = u(x, y, z) - u(a, 6, c). 

For any closed path, W = 0. 

Such a field of force is called conservative. It is true conversely 
that if the field represented by the vector (1) is conservative, 
then there always is a force function, u. For then the integral : 

(*.*. 

(18) u= IXdx + Ydy + Zdz 

(a.b.c) 

is independent of the path and so defines a function u(x,y,z). 
Moreover, 

(19) **, *y, * z . 

dx dy dz 

Potential Energy. When a field of force has a force function, 
u, the negative of u, plus a constant, is defined as the potential 
energy : 

(20) * = - u + C. 
In case, then, a potential <p exists, 



256 MECHANICS 

EXERCISES 

1. Show that the field of force defined by the vector (3) is 
not conservative. But if R be any region of space such that an 
arbitrary closed curve in R can be drawn together continuously 
to a point not on the axis, without ever meeting the axis, though 
passing out of R, then the field of force defined in R by (3) is 
conservative. 

2. A meteor, which may be regarded as a particle, is attracted 
by the sun (considered at rest) and by all the rest of the matter 
in the solar system. It moves from a point A to a point B. 
Show that the work done on it by the sun is 

W = Km(- - 



where r and r x represent the distances of A and B, respectively, 
from the sun, and K is the gravitational constant. 

4. Conservation of Energy. Let a particle be acted on by 
any force whatever. The motion is determined by Newton's 
Second Law : 

(i) ' 

U/l/ U>C/ U/l/ 

Multiply these equations respectively by dx/dt, dy/dt, dz/dt, 
and add : 



dzd^z\ _ ydx , ydy -dz 

} m \dt~dt 2 ~ r ~dt~dt 2 ^ dt ~dfi) ~ dt dt + dt 

The left-hand side of this equation has the value : 

~2dt v *' 
W + ~dP + ~dt 2 ' 



where 

v 2 = 
Hence 



m d 2 Y dx , y, dy t ^ dz 

2 dt dt dt dt 

Each side of this equation is a function of t, and the two func- 
tions are, of course, identical in value. If, then, we integrate 



WORK AND ENERGY 257 

each side between any two limits, < and t lt the results must 
tally : 



f*. v t dt = ( 
J 2dt Vdt J \ 

o 'o 



The left-hand side of this equation has the value : 



The right-hand side is nothing more or less than 
Cxdx + Ydy + Zdz, 

taken over the path of the particle ; 2, (13). But this is pre- 
cisely the work done on the particle by the force that acts. Hence 



The quantity 



mv 



is defined as the kinetic energy of the particle. We have, then, 
in Equation (3) the following theorem. 

THEOREM. The change in the kinetic energy of a particle is equal 
to the work done on the particle. 

If instead of a single particle we have a system of particles, 
the same result is true. For, from the equations of motion of 
the individual particles : 



,.^ d 2 x k v 

(4) mt-^r-Xt, *-- = , 

we infer that 

^ ( v dx k . dy k , dz k 

2( X 



x k . v dy k , 7 dz k \ 

+^ 



The kinetic energy of the system is defined as 



258 MECHANICS 

On integrating, then, between any limits < and < 1; we have 

89 r.-'.- t 

The right-hand side represents the sum of the works done on 
the individual particles, or the total work done on the system. 
The result is the Law of Work and Energy in its most general 
form for a system of particles. 

THEOREM. The change in the kinetic energy of any system of 
particles is equal to the total work done on the system. 

Conservative Systems. In case the forces are conservative; 
i.e. if there exists a force function U such that 



the right-hand side of Equation (5) becomes C/j U g , and so 

(7) 1\ -T = U, - U 
The potential energy, <l>, is defined as : 

(8) $ = - U + const. 
Hence (7) can be written : 

(9) 7 1 ! + * t = T + *o- 
Lett the total energy be defined as 

(10) E = T + *. 
We have, then : 

(11) E, = E m 

or the total energy remains constant. This is the Law of the Con- 
servation of Energy in its most general form for a system of 
particles. 

6. Vanishing of the Internal Work for a Rigid System. Con- 
sider a set of particles which form a rigid system. Let them be 
held together by massless rods connecting them in pairs. Thus 
the internal forces with which any two particles, ra t - and m/, 
react on each other are equal arid opposite : 

(1) F t y + F n = 0, 



WORK AND ENERGY 259 

and lie along the line joining the particles, and furthermore the 
distance between the particles is constant ; i.e. 

(2) rl = ( Xi - xtf + ( yi - 2/y) 2 + (Zi - ztf 

is independent of the time, or 



In general, however, if each particle is connected by these 
rods with all the others, there will be redundant members, so 
that the stresses in the individual rods will be indeterminate. In 
that case, let the superfluous rods be suppressed. 

Consider the work done on the particle mi by the rod con- 
necting it with mj. It is : 



/ 



+ Y^ dyi + Z/ dzi 



and can be expressed by means of the parameter t in the form : 
C( Y { -L- v ^Mi -u 7 ^A ,// 

By the same token, the work done on rn,j by m is 



Since 

Xu + Xn = 0, Ya + Y,-t = 0, Za + Za = 0, 
the sum of these two works can be written in the form : 



i 

/( 



i v (dyi dy\ (dz { dz 

ij ' ~~ + Yii \dt ~ ~ " ~ 



This last integral vanishes. For, the force F i; is collinear with 
the line segment connecting w t - with m jf or : 



Hence the integrand vanishes identically by (3). 



260 MECHANICS 

We have thus obtained the result that the work done by the 
internal forces of a rigid system of particles is nil. It follows, 
then, that the change in the kinetic energy of such a system is 
equal to the work done by the external, or applied, forces. Look- 
ing backward and also forward we can now state the general 

THEOREM. The change in the kinetic energy of any rigid system 
whatever is equal to the work done by the applied forces. 

For a system of particles the proof has been given. Before 
we can extend it to rigid bodies, we must generalize the defini- 
tions of kinetic energy and work. 

6. Kinetic Energy of a Rigid Body. Consider a rigid body. 
Let the volume density, p, be a continuous function. Denote 
by v the velocity of a variable point P of the body. Then the 
kinetiQ energy is defined as 

(i) T = 



extended throughout the region T of space, occupied by the body. 
The vector velocity v of P is the vector sum i) of the velocity 
V along the axis of rotation and ii) the velocity v' at right angles 
to that axis. Hence 

(2) v* = V* + r*a>* 

where r denotes the distance of P from the axis, and co is the 
angular velocity about the axis. Substituting this value in (1) we 
find: 



Hence 

(3) i-Tr+TT 

Let v denote the velocity of the centre of gravity, G ; and lot 
h be the distance of G from the axis of rotation. Then 

0t = F 2 + A 2 co 2 . 
Moreover, 

I = 7 + Mh\ 

where 7 is the moment of inertia about a parallel axis through 
G. Hence 

(4) r 



WORK AND ENERGY 261 

In equations (3) and (4) is contained the following general 
theorem. 

THEOREM. The kinetic energy of a rigid body is the sum of 
the kinetic energy of translation along the instantaneous axis and the 
kinetic energy of rotation about the instantaneous axis. 

It can also be expressed as the sum of the kinetic energy of a particle 
of like mass, moving with the velocity of the centre of gravity, and the 
kinetic energy of rotation about an axis through the centre of gravity, 
parallel to the instantaneous axis. 

One Point Fixed. Let a point of the body be at rest. Let 
the (, 17, f)-axes lie along the principal axes of inertia, being 
the origin. Then the components of the vector velocity v of any 
point fixed in the body are : 

= 770^ fa?,/ 

f w ~~ w 
Vt 

Hence 

(5) T = %(Aw$ 2 + BuJ + Cco^ 2 ). 



If the axes of coordinates are not the principal axes of inertia, 
then 



(6) T = i 

The General Case. From (4) and (5) we infer that 

(7) T = Mv* + (Ap* + Bq* + Cr 2 ), 



where A, B, C are the moments of inertia about the principal 
axes of inertia through the centre of gravity, and p, q, r are the 
components of the vector angular velocity w along these axes. 

7. Final Definition of Work. We have hitherto assumed that 
the point of application, P, of the force is fixed in the body. Sup- 
pose P describes a curve C either in the body or in space. How 
shall the work now be defined? 

Take the time as a parameter. Divide the interval TO ^ t ^ r t 
into n parts by the points = r < t v < - < t n -\ < t n = r v 
Let Qk be the point fixed in the body, which at time t = tk will 



262 



MECHANICS 



reach C ; let Tk be its path in space, and let Vk be its velocity in 
space when it reaches C ; cf . Fig. 120. For the interval of time 



we may take the force as constant, F = F A , the value of F at 

the intersection of I\ with C, and let F* 
act on the point Qk throughout the in- 
terval Atffc. Then J? k will do work equal 
approximately to 




(1) 



F k v k cos \{/ k A^, 



FIG. 119 



where \l/ k is the angle from Tk to F& at 
P k . If Qk is displaced along the tangent 

to T fc a distance v k kt k , the expression (1) represents the work 

precisely. 

We will now define the work as 



F 



Km 



cos 



or, dropping the r-notation and expressing 
the interval of time as t Q g t ^ / t : 




FIG. 120 



(2) 



cf. Fig. 119. In vector form the work is 



W = I Fvcostdt; 



(3) 



! 

= /Fvttt, 

?r 



where v is the vector velocity of Q at P, and Fv is the scalar 
product of these vectors. 

We have used the time as the independent variable, or the 
parameter, in terms of which to define the displacement. But 
the result is in no wise dependent on the time in which the dis- 
placement takes place. Any other parameter, X, would have 
done equally well, provided d\/dt is continuous and positive (or 
negative) throughout. For 

j. ds ,. ds, x 
v at = -TT at = -=- aA. 



WORK AND ENERGY 



263 



This formulation of the definition of work in the general case 
is due to Professor E. C. Kemble. 

Example 1. A billiard ball rolls down a rough inclined plane 
without slipping. Find the work done by ^ 
the plane. 

Here, C is either the straight line or the 
circle; each curve T is a cycloid with 
cusp at P and tangent normal to C ; and 
v = 0. Hence 

W = 0. 




FIG. 121 



Example 2. The same, except that the ball slips. 

The curve C shall be taken along the plane. The normal 

component R = M g cos a does no work ; 

the component along the plane, 




F = 



cos 



does. Let s be the distance travelled 
by the centre of the ball ; 0, the angle 
through which the ball has turned. 
The curve T is a trochoid tangent to C at P. Hence \l/ = or *, 



FIG. 122 



ds 



dd 



and 



' cos {(! s ) - <* (0i - 0o)l- 

Observe that in the definition, Equation (2), v is positive or 0. 
It would not, therefore, be right in this example to write 

_ ds d8 

v ~Tt a dt 

EXERCISES 

1. Check the result in Example 2 by determining the motion 
of the ball and computing the change in kinetic energy. 

2. A train is running at the rate of 40 m. an h. The baggage 
car is empty, and the small son of the baggage master is disport- 



264 



MECHANICS 



ing himself on the floor. He runs forward, then slides. If he was 
running at the rate of 6 m. an h. when he began to slide, and slid 
5 ft., how much work did he do on the car? 

Compute by the definition and check your work by solving 
for the motion. 

3. A rope is frozen to the deck of a ship. The free end is 

^ I haaled , over a smooth pulley at P. 

, **! ^~^~"^ , It takes a vertical component of 

B R = 20 Ibs. to free the frozen part. 

How much work is done ? 

Take the frozen part as straight, and P in the vertical plane 
through it. 

4. Extend the definition of work to a body force, F, where F 
is a continuous vector, defined at each point of the body : 



5. Show that the internal work due to the rope in an At wood 's 
machine is nil. Would this be the case if the rope stretched? 

6. A number of rigid bodies are connected by inextensible 
cords that can wind and unwind on them in any manner without 
slipping. Show that the sum of the works done by the; cords 
on the system and the system on the cords is nil. First, extend 
the definition of work so as to include the case of the work done on 
the system by the part of a cord which is in contact with a body. 

8. Work Done by a Moving Stairway. Consider the work 
which an escalator, or moving stairway, does on a man as he 
walks up. The forces that act on the man are /, S, and Mg, 
where R, S are the components of the 
force which the escalator exerts on his 
foot, and Mg acts at his centre of 
gravity. The curve T is always a 
right line lying in the inclined plane, 
and 

ds 



dt 




FIG. 124 



where s denotes the distance the escalator has moved since the 
man came aboard 



WORK AND ENERGY 265 

The force R does no work, since for it ^ = ir/2. The whole 
work is due to S = F cos ^, and is : 





The speed of the escalator is constant ; denote it by c. Thus 



(2) W 

And 

(3) I = c* t , 

where I is the distance the escalator has moved while the man 
is running up. 

On the other hand, consider the motion of the centre of grav- 
ity of the man. Let the axis of x be taken up the plane. Then 



M --f = S Mg sin a, 



(4) Mu^ Mu = I S dt 



sn a, 



where u dx/dt. 

It follows, then, from (2) and (4) that 

(5) W = c(Mu l MV,Q) + Mgct^ sin a. 

If the man steps off with the same velocity with which he 
stepped on, u^ = w , then, with the help of (3), 

(6) W = Mgl sin a. 

Now 

h = I sin a 

is the vertical distance by which the man would have been raised 
in tho time he was on the escalator if he had not run, but stood 
still. Hence, finally, 

(7) W = Mgh. 

It makes no difference, then, whether the man runs fast or 
slowly, up or down. The one thing that counts is how long he 
is on the escalator. Thus when small boys play on the escalator, 
running up and down, the work the escalator does increases in 



266 MECHANICS 

proportion to the time they are on it, provided they arrive and 
leave with the same velocity. 

9. Other Cases in Which the Internal Work Vanishes. 

i) Two Rigid Bodies, Rolling without Slipping. Here, the 
action and reaction are equal and opposite, though not in 
general normal to the surfaces. Moreover, 
the vector velocity of the point of contact, 
regarded as a point fixed in the one body, 
- - ^p^f - must be the same as the vector velocity of the 
--- ^[ >^ point of contact, regarded as a point fixed in 

V i' v 2 the other body. 

The works done by the two forces Fj, F 2 on 
FIG. 125 the two bodies are : 

*i i 

W 1 = CF.V, cos ft dt, W 2 = (*F 2 v 2 cos ft dt. 




to 



But F l = F 2 , i\ = v 2 , ft + ft = TT. Hence 

W, + W 2 = 0. 

ii) Two Smooth Rigid Bodies, Rolling and Slipping. Here 
the forces F l and F 2 are equal and opposite, and normal to the 
surfaces at the point of contact. The ve- 
locities Vj and v 2 are not equal when there is 
slipping ; but their projections on the normal 
are equal : 

v l cos ft + v z cos ft = 0, 
Since furthermore F l = F 2) we have : 

W 1 + W 2 = 0. Fio. 126 

We have already mentioned the case of rigid bodies on which 
inextensible massless strings wind and unwind, 7, Exercise 6: 
and massless rods were shown in 5 to do no work. Thus syj? 
terns of rigid bodies connected by inextensible strings and rods, 
even though the point of application of the force exerted by the 
string or rod be variable, show no internal work. 

10. Work and Energy for a Rigid Body. THEOREM. The 

change in the kinetic energy of a rigid body, acted on by any forces, 
is equal to the work done by these forces. 




WORK AND ENERGY 267 

We prove the theorem first for two special cases. 

CASE I. No Rotation. Here, the change in kinetic energy is 

m ^i 2 _ -fl^o 2 

w 2 2 ' 

i.e. the change in the kinetic energy of a particle of mass M, 
moving as the centre of gravity is moving. 

On the other hand, consider the work done by one of the 
forces, F : 

(2) W = 

Since there is no rotation, v = v, ^ = ^, 
and 



(3) w = C 



Fvcos$dt. 




Hence W is the work done on a particle at the centre of gravity 
by the same force, and the theorem is true by 4. 

CASE II. One Point Fixed. Here, Eulcr's Dynamical Equa- 
tions, Chapter VI, 13, determine the motion. Consider a force 
F which acts on the body at P. Let r be the vector drawn from 
to P. Then the v of the definition of work, 7, (3) is 

v = & X r. 
Hence 

(4) Fv cos ^ = F - v = F (w X r). 

On the other hand the vector moment of F about is 

From Euler's Equations, I.e., we have : 

A dp . n dq . ~ dr T , ,, , , r 
^TT/ "" '5/ " /it ~ P ' ^ ' ' 
Hence 

(5) $(Ap* + Bq* + 



The left-hand side is the change in kinetic energy. Now 
(6) Lp + Mq + Nr = M - w = co - (r X F), 



268 



MECHANICS 



and so 

(7) Fv cos ^ = Lp + M q + Nr. 

For it is true of any three vectors that 

a - (b X c) + c (b X a) = 0, 



since 



a - (b X c) = 



a 1 a 



Moreover, 
Hence 



w X r =- (r X o>). 

F-(w Xr) = -(r X F). 

From (5) it follows, then, that for a single force, the change 
in kinetic energy is equal to the work done. For the case of 
n forces the proof is now obvious. The extension to the case of 
body forces and forces spread out continuously over surfaces or 
along curves, presents no difficulty. 

Remark. We have shown incidentally that the work done 
on a rigid body with one point fixed is 



h 
J o> t, 



where 

M = La + Mp + Nj 

is the resultant couple. 

The General Case. Consider first a single force, F. The work 
it does is 

W = /Fvd*. 



Here, 

V = V + V', 

where v is the velocity of the centre of gravity and v' is the ve- 
locity of the point Q relative to the centre of gravity, as it flashes 
through P. Hence 

W = 



WORK AND ENERGY 269 



The first integral has the value 

Mv* 



The second integral is equal to the right-hand side of Equation (5). 
Thus the theorem is proved for one force. For a number of 
forces the proof is now obvious. 

EXERCISES 

1. A ball is placed on a rough fixed sphere of the same size 
and slightly displaced near the highest point. Find where it 
will leave the sphere. Let p, have any value. 

2. A weightless tube can turn freely about one end. A smooth 
rod is inserted in the tube and the system is released from rest 
with the tube horizontal. How fast will it be turning when it 
is vertical ? 

3. A cylindrical can is filled with water and sealed up. It is 
mounted so that it can rotate freely about an element of the 
cylinder. Show that it oscillates like a simple pendulum, pro- 
vided the can is smooth. 

4. In the preceding problem, the height of the can is equal 
to its diameter, and the can weighs 5 Ibs. The water weighs 
31 Ibs. Find the length of the equivalent simple pendulum. 

5. A circular tube, smooth inside, plane vertical, is partly 
filled with water. The tube is held fast and the water is dis- 
placed, then released from rest. Show that it oscillates like 
a simple pendulum, and determine the length of the latter. 

6. A bent tube in the form of an L is mounted so that it can 
slide freely on a smooth table. The vertical arm is filled with 
water, and the system is released from rest. How fast will it 
be moving where the vertical arm has just been emptied? 

Assume the tube smooth inside; and also take the weight of 
the tube with its mount equal to the weight of the water. 

7. The can of Question 4 is allowed to roll down a rough in- 
clined plane, starting from rest. Find the acceleration of the 
centre of gravity. 



CHAPTER VIII 
IMPACT 

1. Impact of Particles. Let two particles, of masses m l and 
W 2 , be moving in the same straight line with velocities Ui and 
w 2 , and let them impinge on each other. To find their velocities 
after the impact. 

Isolate the system consisting of the two particles. Then no 
j* 1 w 2 external forces act, and so the 

/$|Q xgfr 

^f u 2 momentum remains unchanged. 

FIG. 128 Hence 

(1) m^ m^! + m 2 u 2 w 2 w 2 = 0. 

As yet, nothing has been said about the elasticity of the par- 
ticles. The extreme cases are: perfect elasticity (like two bil- 
liard balls) and perfect inelasticity (like two balls of putty). 
In each case there is deformation of the bodies for now we 
will no longer think of particles, but, say, of spheres, and the 
velocities u lt w 2 , etc. refer to their centres of gravity. 

During the deformation the mutual pressures mount high, 
and even if other (ordinary) forces act, their effect is negligible, 
compared with the pressures in question. In the case of perfect 
inelasticity, there is no tendency toward a restitution of shape, 
and so, when the maximum deformation has been reached, the 
mutual pressures drop to nothing at all. At this point, the 
velocities of the two centres of gravity are the same, 

u( = u 2 , 

and hence this common velocity, which we will denote by f7, is 
given by the formula : 

(2) u = miUl "*" m * u * 

m l + m 2 

Thus the problem is solved for perfect inelasticity. For partial 
elasticity, it is helpful to picture the impact as follows. The 

270 



IMPACT 



271 



motion of the centre of gravity of each ball is given by the 
equation : 

For the first stage of the impact, i.e. up to the time of greatest 
deformation, t = T, we have, on integrating each side of each 
equation between the limits and T : 

T T 



(4) 



m l u l 



<-T / 

i-o J 



t=T / 

= I J 

/ = e/ 



Rdt. 



The integral is called an impulse,* and is denoted by P : 

T 

(5) P = CR dt. 

o 
Hence 

(6) 



= P 

= P. 



m 2 U 

The second stage of the impact now begins, as the balls are 
kicked apart by their mutual pressures. On integrating the 
equations (3) between the limits T and 7 V , we have : 

T' 

(7) m^ 



fftdt', 



CR'dt'. 



Now it is easily intelligible physically if we assume that, in 
the case of partial elasticity, the value of R' stands in a constant 
ratio to the value of R at corresponding instants of time, or that 



(8) 
when 



R' = eR, 



T - t = t' - T. 



Here the physical constant e is 
called the coefficient of restitution. 
It lies between and 1 : 




t T t' 
FIG. 129 



(9) 



< e < 1, 



* Sometimes spoken of as an impulsive force ; but this nomenclature is unfor- 
tunate, since P is not of the nature of a force, which is a push or a pull, but rather 
is expressed by a change of momentum. Moreover, the dimensions of impact are 
ML/T, not ML/T*. 



272 MECHANICS 

being in the case of perfect inelasticity and 1 for perfect elas- 
ticity. Hence 

7" T 

(10) P' = /V dt f = e CR dt = eP. 

Equations (7) thus yield the following : 

(U) { ^-Ilf/ = df 

The four equations, (6) and (11), contain the solution of the 
problem. Between them, U and P can be eliminated, and the 
resulting equations can then be solved for u[, u 2 . The result is : 



Uf\ : 

* vn.. 4- 

(12)' 



U 2 



m l + m, 2 
e) m 1 u 1 + (ra 2 



The Case m 2 = oo. If in Equations (12) we allow w 2 to increase 
without limit, we obtain the equations : 



U 2 = U 2 . 

These equations do not prove that, when the mass m 2 is held 
fast, or is moving with unchanging velocity u 2 , the velocity of the 
mass m l after the impact will be given by the first equation (13), 
but they suggest it. The proof is given by means of the first 
of the equations (6) and (11), resulting as they do respectively 
from the first of the equations (4) and (7), combined with (10); 
U having here the known value u 2 . 

If, in particular, u 2 = 0, we have : 

(14) u{ = -,. 

Perfect Elasticity, e *= 1. Equation (14) becomes in this case 
u[ = -MI, and the ball recedes with the same velocity as that 
with which it impinged. 

If the masses are equal, m l = w 2 , Equations (12) become : 



IMPACT 273 

and the balls interchange their velocities. This latter phe- 
nomenon can be illustrated suggestively by two equal ivory 
balls suspended side by side from strings 
of equal length, after the manner of two 
pendulums. If one ball hangs vertically 
at rest, and the other is released from 
an angle with the vertical, the second 
ball will be reduced to rest by the im- 
pact, and the first will rise to the same 
height on its side of the vertical as that F 

from which the second ball was released. 

Thus the velocities will be successively interchanged at the lowest 
point of the circular arc. 

Critique of the Hypothesis (8). In this hypothesis we have 
taken for granted an amount of detail in the phenomenon before 
us far in excess of what the physicist will admit as reasonable 
in viewing the actual situation, and he may easily be repelled by 
so dogmatic an assumption in a case that cannot bo submitted to 
direct physical experiment and which, after all, is far less simple 
than we have led the reader to suppose, since the problem is 
essentially one in the elasticity of three-dimensional distribu- 
tions of matter. The objection, however, is easily met. We 
may take Equation (10) : 

P' = eP, 

as the physical postulate governing impact. 

EXERCISES 

1. A ball of 6 Ibs. mass, moving at the rate of 10 m. an h. 
overtakes a ball of 4 Ibs. mass moving at the rate of 5 m. an h. 
Determine their velocities after impact, assuming that the coeffi- 
cient of restitution is . Ans. 7 and 9.5 m. an h. 

2. The same problem, when the balls are moving in opposite 
directions. 

3. A perfectly elastic sphere impinges on a second perfectly 
elastic sphere of twice the mass. Find the velocity of each after 
the impact. 

4. Newton found that the coefficient of restitution for glass 
is ^f . If a glass marble is dropped from a height of two feet 
on a glass slab, how high will it rise? 



274 MECHANICS 

5. In the last question, what will be the height of the second 
rebound? What will be the total distance covered by the marble 
before it comes to rest? * 

6. Find the time it takes the marble to come to rest. 

7. In the experiment with the pendulums described in the 
text, the impinging ball will not be quite reduced to rest, because 
no two material substances are quite elastic. If, for given balls, 
e 0.9, show that the ball which is at rest should be about 11 
per cent heavier than the other one, in order to attain complete 
rest for the latter. What per cent larger should its radius be ? 

8. If, in the last question, the pendulum bobs are of glass. 
e = ^f , find the ratio of their diameters. 

9. If two perfectly elastic balls impinge on each other with 
equal velocities, show that one of them will be brought to rest 
if it is three times as heavy as the other. 

10. Determine the coefficient of restitution for a tennis ball 
by dropping it and comparing the height of riie rebound with 
the height from.which it was dropped. 

11. Some pitchers used to deliver a slow ball to Babe Ruth, 
believing that he could not make a home run so easily as on a fast 
ball. Discuss the mechanics of the situation. 

J 2. Continuation. Oblique Impact. Let two spheres impinge 
at an angle, and suppose them to be perfectly smooth. To de- 
termine the velocities after the 
impact. 

Let the line of centres be taken 
as the axis of x. The deforma- 
tion of each sphere is slight, and 
Fia 131 the force exerted by the other 

sphere, spread out as it ^s over 

a very small area and acting normally at each point of this area, 
will yield a resultant force, K, nearly parallel to the axis of x. 
For the first sphere we have : 

* The physics of the second part of this problem (and of the next) is altogether 
phantastic. After a few rebounds we pass beyond the domain within which the 
physical hypothesis of the text applies, and the further motion becomes a purely 
mathematical fiction. It is amusing for those who have a sense of humor in science. 
But for the literal-minded person, be he physicist or mathematician, it is dangerous. 




IMPACT 275 



(15) 

where 

X = # cos 6, F = 72 sin c, 

e being numerically small and x lt y l referring to the centre of 
gravity, and for the second sphere, 



(16) rn^X, *, F. 

On integrating (15) we obtain : 



,.,,_>. 
(17) 



= - /-Yd*, m,^ 1 ^ = /Yrf*. 

*-o J dl * = o J 



And now we denote the first impulse by P, and lay down the 
postulate that the second impulse is : 



(18) 



Thus the integrals of (15) and (16) load to the equations : 
m^U m l u l = P [ m t F m^^ 



(19) 

1 = P 



which hold for the first epoch of the impact, the equations for 
the second epoch being, as in the corresponding case of 1, the 
following : 

m } u\ m, U = eP { m* v\ m } V = 

1. 
4 m 2 U = eP I m^ m 2 F = 0. 



For we assume as there the physical postulate : 

(21) P' = eP. 

The result at which we have arrived is seen to be the following. 
The component of the velocity of each sphere perpendicular to 
the line of centres has been unchanged by the impact, 

(22) v[ = v l9 v' 2 = v 2 . 



276 MECHANICS 

The components of the velocity along the line of centres are 
changed precisely as in the case of direct impact, 1, Equa- 
tions (12) : 

u\ = - *-- 

mi 
(23) 

Mj = 



m l 



Kinetic Energy. When e l t i.e. when the spheres are per- 
fectly elastic, the total kinetic energy is unchanged by the impact, 
for then 



, 2 _ >\ , 
r ~~ ~ " ~~ ' 



as is shown by direct computation from (23), and the equa- 
tions (22) hold in all cases, whether e = 1 or e < 1. 

When e = 0, i.e. when the spheres are totally inelastic, an easy 
computation shows that the kinetic energy has been diminished. 

The intermediate case, < e < 1, is treated in the same way. 
It follows from direct computation that the left-hand side of 
Equation (24) has the value : 

(m^ + w 2 M 2 ) 2 + m l m z (u l u 2 ) z e 2 



m 2 ) 

and this is at once shown to be less than the right-hand side. 
The terms arising from Equations (22) do not, of course, affect 
the result. 

EXERCISES 

1. A smooth ball travelling south-east strikes an equal ball 
travelling north-east with one-quarter the velocity, their line 
of centres at the time of impact being east and west. If e = ^, 
find the velocities of the balls after impact. 

2. A smooth ball strikes a horizontal pavement at an angle 
of 45. Find the angle of rebound if the coefficient of restitution 
is f. 

3. Show that the kinetic energy of the balls of Question 1 is 
diminished in the ratio of 245/272 by the impact. 

4. The corresponding question for the ball of Question 2. 



IMPACT 



277 



3. Rigid Bodies. Let a rigid body be acted on by a single 
impulse. By that is meant the postulates about to be laid 
down, suggested by the following physical picture. A force F 
acts at a point (x, y) for a 
short time, mounting high in 
intensity. Ordinary forces, if 
present, produce in this inter- 
val of time, ^ t ^ T, only 
slight results, and in the ulti- 
mate postulates do not appear, 

so they are not considered in ^ FrG 132 

the present picture. 

The three equations which govern the motion are : 




- = Y 
dt* *' 



On integrating with respect to the time we find 



(2) 



dt 



M(u' - u) = Cxdt, M(v' - v) = CY 

U 

T T 

7(0' - 0) = Ax - x) Ydt - f(y - y)Xdt. 



Concerning F we will assume that the vector changes con- 
tinuously in magnitude and direction during the interval of 
time in question, and that the point of application, (x, T/), also 
moves continuously, remaining near a fixed point (a, b) through- 
out the interval. Let 

(3) x = a + , y = 6 + 17. 

Then , rj are infinitesimal with T. Let 



(4) 



P = Cxdt, Q = CYdt. 



278 MECHANICS 

The last Equation (2) now becomes : 
(5) /(' - 0) = (a - *) Q - (b - y) P 

T T 

+ CtYdt - Cr,Xdt. 



We should like to infer mathematically that from the hypoth- 
esis that the integrals (4) approach limits when T approaches 0, 
the integrals in the last line of (5) converge toward 0; for then 
we should have the equations : 

M(u'-u)=P, 



(6) ' 7(12' - $2) = (a - x) Q - (b - y) P, 

P and Q here denoting the limiting values of the integrals (4). 

This inference can in fact be drawn, provided the angle through 
which the vector F ranges is less than 180. Equations (6) 
then hold, and, in particular, it follows, on eliminating P and 
Q between them, that 

(7) 7(Q ; - fl) = M(a - x)(v' - v) - M(b - y)(u' - u) 
or 

(8) fc 2 (12' - Q) = (a - x)(v' -v)- (b- y)(u' - u). 

An Example. A rod is rotating about one end, and it strikes 
an obstruction, which brings it suddenly to rest without any 
reaction on the support. What point of the rod comes into 
contact with the obstruction ? 

{Let the distance from the stationary end 
be h, and let I be the length of the rod. 
O k ' Let 

FIG. 133 v = C; then ft = - C. 

Since 

M/ 2 
u = 0, fi' = 0, ^ = 0, 12' = 0, / = ^-, 

we have : 

Hence 

The point is called the centre of percussion. 



IMPACT 



279 



4. Proof of the Theorem. The proof is given by means 
of the Law of the Mean, which is as follows. Let f(x), <p(x) 
be two functions which are continuous in the closed interval 
a ^ x g b, and let <p (x) not change sign there. Then 



ft 

//* 
f(x) <p(x) dx = f(x') I <p(x) dx, a < a:' < 6. 

e/ 



(9) 



In the present case the axes can be so chosen that 

g Y. 

Hence 



(10) 



C^Ydt = ' f*Ydt, 



where ' is the value of at a suitable point, t = ', in the interval 
g g 7 7 . Now, by hypothesis, and T? approach uniformly, 
i.e. the largest numerical value that either has in the interval 
^ t g T approaches 0; and furthermore, also by hypothesis, 
the integral on the right approaches a limit, Q. Hence the inte- 
gral on the left approaches 0. 

If the range of the angle of F does not exceed 90, the axes of 
coordinates can be so chosen that neither X nor Y changes sign 
in the interval ^ t ^ 7 7 , and then it can be shown as above 
that both integrals in the second line of (5) approach 0. 

In the more general case that F is contained merely within 
an angle less than TT, the axes can be chosen in more ways than 
one so that Y will not change sign. 
If (x, y) refer to one such choice and 
(x', y') to a second, then 



(11) 
where 



x' = ax + by 
y r = ex + dy 




FIG. 134 



a = cos 7, b = sin 7, 

c = sin 7, d = cos 7. 
The same transformation holds * with respect to the vector F : 



* It is in such a case as the present one that the scientific importance of the 
proper definition of (-artesian coordinates, laid down in Analytic Geometry, ia 
revealed. That definition begins with directed line segments on a line, proceeds 
to the theorem that the sum of the projections of two broken lines having the same 



280 MECHANICS 

f X' = aX + bY 

(12 > I r-T + fl' 

and also with respect to (, jj) : 

r = of + 6, 



Hence 

r r T T T 

(14) A'*" dt = ac Ax A + 6c Ax dt + bd Cr,Y dt + ad ft-Y dt. 

0000 

The integral on the left, and the last two integrals on the right, 
approach the limit with 7 7 , as has been shown above. We 
will show that this is true also of the other integrals, and hence 
in particular of the last integral in (5). To do this, write down 
Equation (14) for two choices of axes (x f , y') subject to the 
above conditions and characterized by two values of y: y l and 
7 2 , where y l ^ 0, y 2 ^ 0, y l ^ 7 2 , and solve the resulting equa- 
tions for the two integrals in question. The determinant of 
the equations, 



has the value 

sin y l sin y 2 sin (y z - 7^, 

and so does not vanish. Thus the integrals for which we are 
solving are seen to be linear functions of integrals that are known 
to approach 0, and this completes the proof. 

The Restriction. The theorem is not true when F is required 
merely to vary continuously with t in the in- 
terval ^ t ^ T, as the following example 
shows. Let 

X = F cos <?j Y = F sin <p ; 

= p cos ^, 77 = p sin \l/. 
FIG. 135 Then 



extremities, on an arbitrary line, is the same for 'both lines, and ends by declaring 
the coordinates of a point as the projections on the axes of the vector whose 
initial point is the origin and whose terminal point is the point in question. With 
that definition, Equations (12) and (13) are merely particular cases of Equations 
(11), since both sets of equations express the projections of a vector on the coordinate 




IMPACT 281 



Let F and p be constants, and let 

_ 2wt TT _ 2wt 

Then 

r T 

P-fx* Ffa*-0, 









7 1 


7* 


Q=f Yd t = F j 


fc 







r 




yv - ,,2 


)' 








If, now, we set 

__ /TT r __ *_ 

P * > f rpy 

the integrals (4), being always 0, each approach limits, and so 
the P and Q of Formulas (6) have each the value 0. But the 
third Equation (6) does not hold. 

But may it not still be sufficient, in order to secure the vanish- 
ing of the limit of the integral 

T 

/(*r- 



to demand that Y ^ 0? That this is not enough, is shown by 
modifying the above example as follows. Let 

X = F cos ?, Y = 0. 
The integral then has half the value it had before; hence, etc. 

EXERCISES 

1. A uniform rod at rest is struck a blow at one end, at right 
angles to the rod. About what point will it begin to rotate? 

2. A packing box is sliding over an asphalt pavement, when 
it strikes the curbstone. Find the speed at which it begins to 
rotate. 

3. If, in the preceding question, the pavement is icy, and if 
the box, before it reaches the curb, comes to a bare spot, M = 1> 
what is the condition that it should not tip? 



282 MECHANICS 

4. If the box tips, find whether it will slide, or rotate about 
a fixed line. 

6. Show that greater braking power is available when the 
brakes are applied to the wheels of the forward truck of a rail- 
road car. 

6. If all four wheels of an automobile are locked, compare the 
pressure of the forward wheels on the ground with that of the 
rear wheels. 

7. A lamina is rotating in its own plane about a point 0, when 
it is suddenly brought to rest by an obstruction at a point P 
situated in the line OG produced. Show that OP is equal to the 
length of the equivalent simple pendulum, when the lamina 
is supported at and allowed to oscillate under gravity in a 
vertical plane. 

5. Tennis Ball, Returned with a Lawford. Consider a tennis 
ball, returned over the net with flat trajectory arid rotation such 
that the lowest point of the ball is moving backward. The 
ground thus exerts a forward force, and we will assume that this 
state of affairs holds throughout the impact. We shall have, 
then, the following formulation of the problem : 

M(U - M ) = Q Mfa - {/) '== eQ 
M(V -V Q ) = Q M(v, - F) = eQ 




where 

^^^^ no 

F=pR 
Fid. 136 

is the impulse. First of all, 

V = 0, 

for the point of greatest deformation is marked by the centre 
of gravity of the ball's ceasing to descend. Thus we have seven 
equations for the seven unknowns, u { , v lt co t , [/, V, 12, Q. 
It is now easy to solve. Observe that 

V Q < 0, co < 0, u > 0. 



IMPACT 283 

We have, then : 

Q = M(- t> ), v l = e(- V Q ), 



The value of c^ is not interesting. What we do want to know is 
the slope of the trajectory at the end of the impact ; i.e. 

v __ _ e( VQ) _ __ _ e\ _ 
^ " u + (1 + e ) M (-t, ) ~ 1 + (1 + e)/i\ f 

where X = ( VQ)/U Q is the numerical value of the slope before 
the impact. 

As the ball has a drop due to the cut, X will be considerably 
larger numerically than the slope in the part of the trajectory 
just preceding the last ten feet or so before touching the ground. 
It might conceivably have a value as great as . The value of 
e is about 0.8. ju varies considerably and might be as high as . 
Thus 

& = .15, 
*i 

as against X = .20, or the steepness of the rebound is only three- 
fourths the steepness of the incident path. 

Not only does the ball rise at a smaller angle, but the horizontal 
velocity is increased by nearly 10 per cent ; for 

u, = w [l + (1 + <0/*A] = 1.09t* . 

For this discussion to be correct it is essential that the ball 
maintain its spin throughout the whole impact. This explains 
the nature of the stroke. The racquet has a high upward velocity 
while the ball is on the guts. 

The ball loses spin during the flight before the impact, due to 
the air resistance causing the drop, and this loss may easily be 
comparable with the loss during the impact. It would be inter- 
esting to take motion pictures of the ball, showing the trajectory 
just before and just after the impact. 

EXERCISES 

1. A billiard ball, rotating about a horizontal axis, falls on 
a partially elastic table. Find the direction of the rebound if 
ju = % and e = .9. 



284 MECHANICS 

2. A rod, moving in a vertical plane, strikes a partially elastic 
smooth table. Determine the subsequent motion. 

3. The preceding question, with the change that the table is 
rough, M = i- 

4. Question 2 for a table that is wholly inelastic and infinitely 
rough. 

5. A rigid lamina is oscillating in a vertical plane about a 
point when it strikes an obstacle at P whose distance from 
is equal to the length of the equivalent simple pendulum. Show 
that it will be brought to rest without any reaction on the axis. 

For this reason P is called the centre of percussion. 

6. A rigid lamina, at rest, is struck a blow at a point 0. Find 
the point about which it will begin to rotate. 

7 % A solid cone, at rest, is struck a blow at the vertex in a 
direction at right angles to the axis. About what line will it 
begin to rotate ? 




CHAPTER IX 
RELATIVE MOTION AND MOVING AXES 

1. Relative Velocity. It is sometimes convenient to refer the 
motion of a system to moving axes. Let O be a point fixed 
in space. Let 0' be a point moving in any manner, like the 
centre of gravity of a material body, or the centre of geometric 
symmetry of a body whose centre of gravity is not at 0'; it is 
a point whose motion is known, or on which we wish particularly 
to focus our attention. Finally, let P be any point of the system 
whose motion we are studying. Then 

(1) r = r + r', 

dr _ dr di^ 
dt " dt ^ dt' 
or 

(2) v = v + v'. 

, i , i FlG - 137 

The choice of notation is here particularly 

important boldface letters denote as usual vectors because 
we have two analyses to emphasize, namely, i) the breaking up 
of the velocity v into the two velocities v and v'; and if) the 
breaking up of v' into the two velocities : 

(3) v' = v r + v., 

where v r , the relative velocity, and v e the vitesse d'entrainement are 
presently to be defined. For this purpose we must first recall 
the results of an earlier study. 

2. Linear Velocity in Terms of Angular Velocity. In Chap- 
ter V, 8, we have studied the motion of a system referred to 
moving axes (, 17, f ) with fixed origin 0. Here, 

(4) r = a + iff + f y 
and 



+ r/4 + f 7- 
285 



286 



MECHANICS 



This equation represents an analysis of the velocity 

(6) v = 

of the point P into two velocities, namely, 

(7) v = v r + v e , 
where 

(%} v = 4- #4-^ 

is the relative velocity of P with respect to the moving axes ; i.e. the 
absolute velocity which P would have if the ( , r;, f )-axes were 
at rest and the point P moved relatively to them just as it does : 

(9) = f(t), ?? = <p(t), f = \l/(i). 
Secondly, 

(10) V e = a + rift + f 7 

is the vitesse d'entrainement, the Schleppgeschwitidigkeit, the 
velocity with which that point Q fixed in the moving space and 
flashing through P at the one instant, t, is moving in space. Let 
(w) be the vector angular velocity of the moving axes : 

(11) (w) = pa + qp + ry, 
where 

Then 

(12) v e = () X r, 




FIG. 138 



or 
(13) 



+ (& - f p) j8 + (77?? - 



y. 



The final result is as follows : The components of v, or dr/dt, 
along the axes are 



(14) 



RELATIVE MOTION AND MOVING AXES 287 

I repeat : These are the formulas when the moving axes 
have their origin, 0', fixed : r = 0, v = 0, v = v'. 

3. Acceleration. Returning now to the point P of 1 and 
Equations (1) and (2), we define its acceleration as the vector: 



Hence 

(16) a = + , 
or 

(17) a = a + a'. 

The first term on the right, a , requires no further comment. 
It is merely the acceleration in fixed space of the known point 0'. 
The second term, a', relates to the rotation and admits of a num- 
ber of important evaluations. 

First Evaluation. The first of these is as follows. Let a' be 
denoted by a. Then 

< -T 

We may identify the variable vector v' with the variable vector 
r of 2, Formula (4) ; for, of course, r was any vector, moving 
according to any law we wish. Now, we have evaluated the 
right-hand side of (18) by means of Equations (14). Hence the 
components of the right-hand side of (18) are obtained by sub- 
stituting in the right-hand side of (14) for , rj f f respectively 

v > v ^ v - 

On the other hand, write 

(19) a = a$ a + a^ ft ~f~ fl <7- 

Thus wo arrive at the final determination of a in terms of known 
functions : 

__ dv* * __ 



(20) 



dVrt 



= ~ 



a$ jT- + pity qv$ 
These are the formulas referred to as the First Evaluation. 



288 MECHANICS 

Second Evaluation. The Theorem of Coriolis. Another form 
for the vector a can be obtained by differentiating (5), 2 : 



+ f + 77/3 + f y. 
Thus 



o | _ 

y* dt ! c^ l <ft e&y 

+ <* + r/j3 + f 7. 

This result is due to Coriolis. 
The first and third lines admit immediate interpretations. For, 



is the relative acceleration, or the acceleration of P referred to the 
(> Vy f)-axes as fixed. Next, 

(23) ae== ^ + 77 d^ + f W~ 

is the acceleration d'entrainementj or the SchleppbesMeunigung, 
the acceleration with which the point Q, fixed in the moving 
space and coinciding at the instant t with P, is being carried 
along in fixed space. 
The vector (23) : 

a e = & + tip + fy, 

can be computed as follows. Since as is geometrically, or 
kinematically, immediately obvious 

(24) a = r/3 - qy, $ = py - ra, y = qa - p/3, 
we have : 

(25) -J-} 

+ rp - qy. 
The last line has the value : 



RELATIVE MOTION AND MOVING AXES 289 

where 

(co) = pa + q@ + ry. 

Hence 

/oc\ / \dQ dr\ f.dr >.dp\ / dp 

(26) * - r - ' a + - f ' + " - 



- w 2 ( + i?/3 + r 7) + (p$ + qr> + rf)(pa + g/8 + ry), 
or 

(27) a e = (0 X r - 2 r + (()r) (), 

where 



This vector (w') is the velocity relative to the fixed axes (, 77, f), 
with which the terminal point of (co) is moving when the initial 
point is at 0' ; it is the relative angular acceleration, referred to the 
(> *?> f )-axes as fixed. 
Finally, the vector 



a = 
' dtdt^ dtdt^ dt dt j 

can be expressed in the form : 

(30) a = (co) X v r , 

or: 



For, on recurring to Formula (10) of 2 and taking, as the arbi- 
trary vector r, the vector v r , which is given by (8), the right- 
hand side of (10) comes to coincide with the right-hand side of (29). 
With the aid of (12), this vector can be written in the form of the 
right-hand side of (30), and this completes the proof. 

To sum up, then : From (17), 

(31) a = a + a', 

where a' = a, and a is given by (20). A second evaluation of a 
is given by (21), 

(32) a = a r + 2a t + a e , 

where a r is given by (22) and a c by (23) ; the latter, in a differ- 
ent form, by (26) or (27). Finally, a t is given by (29) or (30). 



290 MECHANICS 

4. The Dynamical Equations. From Newton's Second Law of 
Motion, written in the form : 

(1) ma = F, 
it follows that 

(2) ma + ma = F, 

where a is the acceleration of the moving origin, 0', and 
a = a r + 2a, + a*. 

The vector a r is the relative acceleration and is given by For- 
mula (22), 3. The vector a c is the acceleration d' entrainement 
and is defined by (23) ; it is represented by (26) or (27). Finally, 
a* is defined by (29) and is represented by (30). 

If the motion of the moving axes is regarded as known, then 
Q O is'a known function of t t and (o>), i.e. p, q, r are known from 
(11), 2. Equation (2) can now be written in the form : 



(3) ma r = F ma Q 2ma ma e . 

On substituting for a* its value from (30) and for a e its value 
from (26), a system of differential equations is found for deter- 
mining , 77, f : 

rf \dt dt dt 

(4) 



where the functions /, <p, \l/ can be written down explicitly from 
the above formulas. 

More generally, Equation (1) can be thrown into the form 
required in a given problem by using a suitable form for a, a , 
a r , a^ a as pointed out at the end of 3. Each one of these 
accelerations must be studied in the particular case. There is 
no single choice of sufficient importance to justify writing down 
the long formulas. But the student will do well to make hi^ 
own syllabus, writing down the value of a r and each form foi 
a,, a { . 



RELATIVE MOTION AND MOVING AXES 291 

EXERCISE 

Obtain the dynamical equations in explicit form from La- 
grange's Equations, Chapter X. Observe that 

f 6? + & f p + tfop) 2 



where 



_ __ 

Vy ~ V ' 7 - * 3 -ft- + * -fa + "I -5- 

5. The Centrifugal Field. Let space rotate with constant 
angular velocity about a fixed line through 0, the (, rj, f)-axes 
being fixed in the moving space. Then the vector angular 
velocity (o>) is constant, and a = 0. The vector a e , 3, (27) 
reduces to : 

(1) a.=-*r+(().r)(), 

and is easily interpreted. Kinematically, it is, of course, the 
centripetal acceleration ; geometrically, it is a vector drawn from 
the point P toward the axis and of length o> 2 p, where p is the 
distance from P to the axis. 
Newton's Law takes the form : 

ma = F, 

where a is given by 3, (32), and thus 



(2) a = + 2q - 2r - + pfa + 9, + rf ) 



292 



MECHANICS 



Axis of f, the Axis of Rotation. In this case, 
r = w, and the equations reduce to the following : 



(3) 



p = q = 0, 




Fia. 139 



Thus the motion along the axis of f is the same as it would 
be if space were not rotating. The projection of the path on 
the (, 77)-plane is the same as the path of a particle in fixed, or 
stationary, space, when acted on i) by the applied force F ; ii) by 

a force rao> 2 /> directed away from ; 
and Hi) by a force at right angles to 
the path, equal in magnitude to 2ma)V, 
and so oriented to the vector velocity 
v as the positive axis of is, with re- 
spect to the positive axis of 17. 

This third force is known as the 
Coriolis force. In the case of the 
Centrifugal Oil Cup, and the corre- 
sponding revolving tennis court, Chapter III, 23 it was enough, 
for problems in statics, to take into account the u centrifugal 
force," or the force ii) above. But for problems in motion, this 
is not sufficient. There is the Coriolis force Hi) at right angles 
to the path, like the force an electro-magnetic field exerts on a 
moving charge of electricity. 

6. Foucault Pendulum. Consider the motion of a pendulum 
when the rotation of the earth is taken into account. We may 
think, then, of the earth as rotating about a fixed axis through 
the poles, which we will take as the axis of z, the axes of x and y 
lying in the plane of the equator. 

Let P be a point of the northern hemisphere, and let its dis- 
tance from the axis be p. By the vertical through P is meant 
the line in which a plumb bob hangs at rest, or, more precisely, 
the normal to a level surface. Let f be taken along the vertical, 
directed upward; let be tangent, as shown, to the meridian 



RELATIVE MOTION AND MOVING AXES 293 

through the point of support of the pendulum; then 77 will be 
tangent to the parallel of latitude through the point of support, 
and directed west. Let X be the latitude of P; i.e. the angle 
that f makes with the plane of the 
equator. 

The earth rotates about its axis 
from west to east, and so the 
vector angular velocity, (co), is 
directed downward. Thus 

p = co cos X, q = 0, 
r = w sin X, 
2rr 



co = 



24 60 - 60 



= .000727. 




FIG. 140 



We can now write down the differential equations that govern 
the motion. These are contained in the single vector equation 

of 4 : 

ma + ma = F. 

Let P be the point of support, and let (f, 1?, f ) be the coordinates 
of the pendulum ; Z, its length, 

First, compute F : 

F = G + N, 
where 

- au , w.c>u 



is the force due to gravity, or the attraction of the earth ; and 
N = - j^a-Jtffl- j-#7 

is the tension of the string. 
Next, a is the centripetal acceleration, or : 

a = co 2 p( sin X + 7 cos X). 

Finally, a is given by the formulas (2) of 5. For, although 
these were written down for the particular case a = 0, they apply 
generally, where a is arbitrary, provided the vector angular 
velocity of the moving space is constant. 

Thus we can write down explicitly the three equations of mo- 
tion. These we replace by approximate equations obtained as 



294 MECHANICS 

follows. Approximate, first, to the field of force by the gravity 
field. 



field, 

U = - 



U = - mg . 

Next, suppress those terms which contain co 2 as a factor, or are 
of the corresponding order of small quantities. Thus 



Finally, 

? + T? + f 2 = 



= -I + r? + terms of higher order. 






We introduce the further approximations which consist in sup- 
pressing the term in d/dt in the second equation, and setting 
N = mg. The first two equations thus become : 



A) 



Discussion of the Equations. Multiply the first equation A) 
through by di/dt, the second by dq/dt, and add. The resulting 
equation, 



, 
dtdt*~^dtdt* 

integrates into the equation of energy : 



2~ Z 2 
or, on introducing polar coordinates, 



RELATIVE MOTION AND MOVING AXES 295 

Next, multiply Equations A) by j and respectively, and 
subtract : 



This integrates into 

drj d _ , 2 r 
%- 17 ^- cor + C ' 
or 

(2) fJ = 'r + C f 

where co' = sin X. 

4 Special Case. Let the pendulum be projected with a small 
velocity from the point of equilibrium. Then initially r = ; 
hence C = and 

dB 

di = "' 
It follows, then, that 

= w't. 

This means that, if the motion be referred to moving axes, so 
chosen that f' coincides with f, but ' makes an angle u't with , 
the pendulum will swing in the (', f ')-plane. It is now easy to 
determine r as a function of t from (1) ; r executes simple harmonic 
motion. 

The General Case. Returning now to the general case, let 
the motion be referred to a moving plane through (the point 
of equilibrium of the pendulum), perpendicular to the f-axis, 
and rotating with constant angular velocity a/ about 0. Then 

(3) <f> = B - u't 

is the angular coordinate in the new plane. Equation (2) now 
becomes : 

(4) r-l-C, 

and this is the equation of areas in its usual form. 
Equation (1) goes over into : 



or 

(5) ^ + r^ + 2'C + rV = - |r 2 + . 



296 MECHANICS 

On suppressing the term r 2 ' 2 because of its smallness, we find : 

+--!-+* 

But this is precisely the equation of energy corresponding to an 

attracting central force of intensity -y^r. Hence the motion 

I 

is elliptic with at the centre ; i.e. the pendulum, once released, 
describes a fixed ellipse in the moving plane. The axes of this 
ellipse rotate in the positive sense, i.e. the clockwise sense, as one 
looks down on the earth. But the pendulum describes the ellipse 
in either sense, according to the initial conditions, the degenerate 
case of the straight line lying between the description in positive 
sense and that in negative sense. In the Foucault experiment 
in the Pantheon the pendulum was slightly displaced from the 
position of equilibrium and released from rest relative to the 
earth. It then described the ellipse in the negative sense. For 
initially dr/dt was 0, so that it started from the extremity of 
an axis (obviously the major axis) and its initial motion rela- 
tive to the moving plane was in the negative sense of rotation ; i.e. 
counter clockwise. At the end of twenty-four hours, t has the 
value : t = 24 X 60 X 60, and hence 

= u't = 27rsinX. 

The result checks, for at the equator should be 0, and at the 
North Pole, 2w. 

EXERCISE 

Obtain the equations of motion A), directly from Lagrange's 
Equations, Chapter X. 



CHAPTER X 
LAGRANGE'S EQUATIONS AND VIRTUAL VELOCITIES 

INTRODUCTION 

In the preceding chapters, the treatment has been based on 
Newton's Second Law of Motion. Work and Energy have 
entered as derived concepts. It is true that certain general 
theorems have been established, whereby some of the forces of 
constraint have been eliminated, like the theorem relating to 
the motion of the centre of gravity, and the theorem of rotation of 
a rigid body. But in the last analysis, when there have been forces 
of constraint which have not annulled one another in pairs, the 
setting up of the problem has involved explicitly any unknown 
forces of constraint, as well as the known forces, and the former 
have then been eliminated analytically, anew in each new problem. 

We turn now to methods whereby, in certain important cases, 
the forces of constraint can be eliminated once for all, so that 
they will not even enter in setting up the equations on whose 
solution the problem depends. Moreover, we introduce intrinsic 
coordinates and intrinsic functions. The intrinsic coordinates are 
a minimum number of independent variables whose values locate 
completely the system. They are often called generalized coordi- 
nates, and are denoted by q lt , q m . The intrinsic functions are 
the kinetic energy, the work function or its negative, the potential 
energy, and the Lagrangean function L. These we have called 
intrinsic because they do not depend on any special coordinate 
system, or on any special choice of the q's. Later, we shall consider 
intermediate cases in which the number of q's, though highly re- 
stricted, is not a minimum, and in which, moreover, the unknown 
forces, or constraints, have not been wholly eliminated. 

1. The Problem. A material system may be determined in 
its position by one or more coordinates, q lt - , </,* and the 

* We choose, in general, the letter m to denote the number of the q's. But we 
replace it by n in these early examples to avoid confusion with the m that refers 
to the mass of the particle. 

297 



298 MECHANICS 

time, t. For example, let a bead of mass m slide freely on a 
smooth circular wire, which rotates in a horizontal plane about 
. one of its points, 0, with constant angular 
velocity. The angle <p that the radius 
drawn from makes with a fixed hori- 
zontal line is given explicitly, 




Let 9 be the angle from OQ produced to 
the radius, QP 9 drawn to the bead. Then 

the position of m is fully determined by 6 and t. Thus if we 

set = q, 

x = f(q, t), y = \(/(q, t). 

The problem of determining the motion is that of finding q 
as a function of t. 

More generally, let a smooth wire, carrying a bead, move 
according to any law, and let the bead be acted on by any forces. 
To determine the motion. We will treat this prob- 
lem in detail presently. 

As the second illustrative example, consider n 
masses, m l9 , m nj fastened to a weightless in- 
extensible flexible vstring, one end, 0, of which is 
held fast, and let the system be slightly displaced 
from the position of equilibrium. To determine the m j 
oscillation. 

Finally, we may think of a rigid body, acted on 
by any forces. If there are no constraints, it will 
require six coordinates, q lt q z , , q B9 to determine 
the position. These may be the three coordinates 
of one of the points of the body, as the centre of 
gravity, x, ?/, 2; and the three Eulerian angles, 
0, tp 9 \f/ 9 which determine the orientation of the 
body. 

We may, however, also introduce constraints. If 
one point is fixed, there are three degrees of free- 
dom, and so three coordinates, q l9 </ 2 , q Z9 for ex- / 
ample, the Eulerian angles are required. Or, 
again, the body might rotate about a fixed axis. 
Then n = 1, and q l = q 9 a single coordinate would be 
sufficient. Or, finally, the body might be free to slide along 




LAGRANGE'S EQUATIONS. VIRTUAL VELOCITIES 

a fixed line and rotate about it. Here n = 2 and q lf q are the 
coordinates. 

Each of the last two examples may be varied by causing the 
line to move in an altogether specified manner. Then, beside 
q l = q, or q 1 and q 2 , the time, t, would enter explicitly. 

In all such cases, the motion is determined by Lagrange's 
Equations, which, when there is a force function U, take the 
form: 

A\ 1(1 T _^-^ _ i 

A; dtdb dq~,~dq r ' r-1, ...,m, 

where T denotes the kinetic energy, and q r dq r /dt. We turn 
now to the establishment of these equations, beginning with the 
simplest cases. 

2. Lagrange's Equations in the Simplest Case. Let a bead 
slide on a smooth wire whose form as well as position varies with 
the time : 

(1) x=f(q,f), */ = *>(<?, 0, * = *(</,*), 

where the functions f(q, t), <p(q, t), \f/(q, t) are continuous to- 
gether with whatever derivatives we need to use, and where 

fa 8y dz 

V 'dq' dq 

do not all vanish simultaneously. The motion is determined by 
the equations : 

" 



(2) 



where X, F, Z refer to the given, or applied forces, i.e. forces 
other than the reaction, (X, Y, Z), of the wire, and 

(3) XX + /*Y + v1 = 0, 

where (X, /z, v) are the direction components of the tangent to 
the wire for the reaction of the wire is normal to the wire, 
though otherwise unknown. 



300 MECHANICS 

Multiply these equations through by dx/dq, Sy/9q, 8z/8q re- 
spectively and add : 



8y Pz8z\ _ 
^ + dt* dq) ~ y> 



the remaining terms, namely : 

y dx . y dy 7 dz 

A TT~ i "o~ i *- ~^r~i 

dq dq dq 

vanishing because of (3), since dx/dq, dy/dq, dz/dq are the di- 
rection components of the tangent to the wire. 

The left-hand side of Equation (4) can be transformed as 
follows. We write : 

tYI 

(6) T = ~ (x* + y* + z*) 9 

where the dot notation means a time derivative : 

dx . dq . 

x = Tt> ^Tv ctc - 

From (1) 



dx _ 

dt ~ dqdt " dV 
or 

/\ . dx . . dx 

(7) ^ITqO + Jt' 

with similar expressions for y and z. On substituting these 
values in (6), T becomes a function of q, q, t. And now the left- 
hand side of Equation (4) turns out to be expressible in the form : 

<W <L d L-?L 

W dt dq dq 

For, first, we have : 



dT f.dx..dy..ai\ 
-z-r = m[x + y-~ + z~). 
dq \ dq dq dq/ 



From (7) it follows that 

dx = dx 
dq ~ dq 



LAGRANGE'S EQUATIONS. VIRTUAL VELOCITIES 301 

with similar expressions for dy/dq and dz/dq. Thus 
dT 



Next, differentiate with respect to the time : 
.V d dT __ /d 2 x dx d 2 y dy d 2 



' dtdq \dt 2 dq dt 2 dq dt 2 dq, 

. / . d dx . . d dy . d < 

On the other hand, 

dT _ / . dx _j_ . dy L . dz 
_ _ m ^ 

Now, 



, 1AN 

(10) = ^-. 

dq \ dq dq dq/ 



dx _ d dx 
'dq ~ dt~dq' 
For, from (7), 

f)'V s)^ IF /ft IT 

UJU (/ JU . . C/ JU 

~dq ~ ~dif q dqdt' 
and, of course, 

d dx d 2 xdq d 2 x 

Jt~dq = d^~dt dtdq' 

Substituting the value given by (11) and the corresponding 
values for dy/dq, dz/dq in the right-hand side of (10), we see 
that dT/dq is equal to the last half of the right-hand side of (9), 
and thus the proof is complete : the left-hand side of (4) has 
the value (8). We arrive, then, at the final result : 



- 
dt^j 8q ~ ' 

This is precisely Lagrange's Equation for the present case. 

The case that the applied forces have a force function, U, is of 
prime importance in practice. Here 



dV v dU 8U 

~> Y = '' ~' 



and thus Q becomes : 



= 4. 4. . 

dx dq dy ~dq "*" dz dq 



302 MECHANICS 

Lagrange's Equation now takes the form : 



dt dq dq dq 

Example. Consider the problem stated at the opening of the 
paragraph. Here, the applied forces are absent, and so U = const. 
Furthermore, 

x = a cos ut + a cos (6 + coJ) 

y = a sin ut + a sin (0 + ui) 
where q = ; and 

x = aco sin ut a (0 + co) sin (0 + co) 
2/ = aco cos to + a (^ + co) cos (^ + co<) 

T = ^- ((^ + a?) 2 + 2co(0 + co) cos + co 2 ) 
orn /^T 1 

r = ma 2 (^ -f co + co cos 0), = ma 2 co(0 + co) sin 0, 
d dT 3T /d*B , o . 

5ay"-8 a " ma "(3i +w8i 

or 

g=-.. dn , 

This last is the equation of Simple Pendulum Motion, 

d*Q g ^ 

-& }**' 

Thus the bead oscillates about the moving line OQ as a simple 
pendulum of length 

Z - 

^~co 2 

would oscillate about the vertical. 

EXERCISES 

1. A bead slides on a smooth circular wire which is rotating 
with constant angular velocity about a fixed vertical diameter. 

Show that 

tl^fi 

-^ = co 2 sin 6 cos B + 2 s i n 0. 

at* a 



LAGRANGE'S EQUATIONS. VIRTUAL VELOCITIES 303 

2. If the bead is released with no vertical velocity from a 
point on the level of the centre of the circle, show that it will 
not reach the lowest point if 



3. A bead slides on a smooth rod which is rotating about 
one end in a vertical plane with uniform angular velocity. Show 
that d2r 

= w 2 r + g sin wt. 

4. Integrate the differential equation of the preceding ques- 
tion. 

6. A bead slides on a smooth rod, one end of which is fixed, 
and the inclination of which does not change. Determine the 
motion, if the vertical plane through the rod rotates with constant 
angular velocity. 

6. In the problem discussed in the text, determine the reac- 
tion, N, of the wire. Ans. N = ma 2 [w 2 cos 6 + (0 + w) 2 ]. 

7. A smooth circular wire rotates with constant angular 
velocity about a vertical axis which lies in the plane of the circle. 
A bead slides on the wire. Determine the motion. 

8. Show that if, in Question 1, the axis is a horizontal di- 
ameter, the motion is given by the equation : 

~~ f w 2 cos (p + ~ cos coH sin <p = 0, 

where <p is the angle which the radius drawn to the bead makes 
with the radius perpendicular to the axis. 

9. A bead can slide on a smooth circular wire which is expand- 
ing, always remaining in a fixed plane. One point of the wire is 
fixed, and the centre describes a right line with constant velocity. 

Determine the motion of the bead. . , 8 

Ans. 6 = a + - 
t 

10. The same problem if the centre is at rest and the radius 
increases at an arbitrary rate. 

3. Continuation. Particle on a Fixed or Moving Surface. Let 

a particle, of mass w, be constrained to move on a smooth sur- 
face, which can vary in size and shape, 

(1) x = f(q l9 q 2 , 0, V 



304 MECHANICS 

where the functions on the right are continuous, together with 
whatever derivatives we wish to use, and the Jacobians 



do not vanish simultaneously. The motion is given as before by 
Equations (2) of 2, where now, however, the reaction, due to 
the surface, is known in direction completely. 

Multiply these equations through respectively by Sx/dq l9 
dy/d<li, dz/d<li> and add. On the right-hand side there remains 
only 



since dx/dq lf etc. are the direction components of a certain line 
in the surface, drawn from (x, y, z), and X, Y, Z are the com- 
ponents of a force normal to the surface. Hence 



* dq, dt* dq, * 

The reduction of the left-hand side is similar to the reduction 
in the earlier case. It is, however, just as easy to carry this 
reduction through for a system with n degrees of freedom, and 
this is done in the following paragraph. Thus we see that 



dt dq t dq l l ' 
and, similarly : 

dt dq% dq% 

These are Lagrange's Equations for the case of two variables; 
i.e. the case of (q l9 q z ). If, in particular, a force function, [/, 
exists, then Lagrange's Equations take the form : 

\ d (/ 2 u L uLJ d u L u L uU 

dt dqi dq l dq dt dq 2 ^2 ^2 

Example. A particle is constrained to move, without fric- 
tion, in a plane which is rotating with constant angular velocity 
about a horizontal axis. Determine the motion. 



LAGRANGE'S EQUATIONS. VIRTUAL VELOCITIES 305 

Let the axis of rotation be taken as the axis of x, and let r 
denote the distance of the particle from the axis. The coordi- 
nates of the particle are (z, y, z), 
where 
y = r cos 0, z = r sin 0, = co, 

and we take q l = x, q 2 = r. Then 
y r cos w 7*w sin co, 
z r sin o>2 + rw cos ait, 



a result that may be read off directly, without the intervention 
of y, z. Furthermore, 

U = mgz = mgr sin ut. 
Lagrange's Equations now become : 

dT . dT n dU n 

-r-r = mx, ~^~ = 0, - = 0; 

dx dx J dx 




a result immediately obvious. Next, 
dT . dT 



or 



= mg sin < 
ttr* mco 2 r = ing sin co/, 

^2 - o> r =-^sm^. 



A special solution of this equation is found, either by the method 
of the variation of constants or, more simply, by inspection, to be : 



sni 

r 



" 2co 
Hence the general solution is 



Since = w^, the equation can be written in the form : 



306 MECHANICS 

A particular case of interest is that in which A = B = 0. 
This corresponds to the initial conditions of launching the particle 
from a point in the axis with a velocity whose projection along 
the axis is arbitrary, the projection normal to the axis being g/2w. 
The path is then a helix. 

EXERCISES 

1. A cylinder of revolution is rotating with constant angular 
velocity about a vertical axis, exterior to the cylinder, the axis 
of the cylinder being always vertical. A particle is projected 
along the inner surface, which is smooth. Determine the motion. 

2. Use Lagrange's Equations to determine the motion of a 
particle in a plane, referred to polar coordinates : 

d*r dd*\ md 



4. The Spherical Pendulum. Consider the spherical pendu- 
lum ; i.e. a particle moving under gravity and constrained to lie 
on a smooth sphere. Take as coordinates the colatitude, 6, and 
the longtitude, <p, the north pole being the point of unstable 
equilibrium . Then 

fY)f]1 

T = ^- (02 + p S i n 2 0)^ jj = _ mfif2 = _ mga cos e . 



O/TI PT 7 %TT 

- = ma 2 6, = ma 2 <f> 2 sin 6 cos 0, - = mga sin 0, 

00 Cv Cv 

and the first of Lagrange's Equations becomes : 

ma 2 S ma 2 (f> 2 sin 6 cos 6 = mga sin 0, 
or 



a 
Proceeding now to the second equation, we have : 



Hence 



LAGRANGE'S EQUATIONS. VIRTUAL VELOCITIES 307 

This equation integrates into 
(2) ^sin*0 = h, 

where the constant h is of dimension 1 in the time, [T~ 1 ]. 
Combining Equations (1) and (2), we obtain: 

- 



This is the Equation of Spherical Pendulum Motion. In case 
the motion is to be studied for small oscillations near the lowest 
point of the sphere, it is well to replace 6 by its supplement, 
6' TT 6. Equation (3) then becomes : 



This last equation reduces to the Equation of Simple Pendulum 
Motion when h = 0. Any differential equation of the form : 

fA\ d 2 6 A cos0 D . 

(4) r = A --T-T + B sm 6, 

at 2 sm 3 6 

where A > and B > are arbitrary constants, can obviously 
be interpreted in terms of spherical pendulum motion. 

A first integral of (3) can be obtained in the usual manner : 



2A 2 cosgdfl 2g . dfi 
dtdP sin 3 dt "*" a * m dt' 

Integrating each side with respect to 0, we obtain : 

< --;-?- + * 

For a further discussion of the problem, cf. Appell, Mecanique 
rationelk, vol. i, 277. 

EXERCISES 

1. Give an approximate solution for small oscillations near 
the point of stable equilibrium, 0, using Cartesian coordinates. 
Here, 



and the approximate path is an ellipse with as centre. 



308 MECHANICS 

2. Treat the motion of a particle constrained to move on a 

smooth surface, 2 

22 = a 2 2 + 2 2/ 2 , 

for small oscillations near the origin. 

3. Show that a top which is not spinning moves like a spherical 
pendulum. More precisely, we mean the body of Chapter VI, 
18, when v = 0. 

6. Geodesies. Let a particle be constrained to move on a 
smooth surface under no applied forces. The path is a geodesic.* 
Let the surface be given by the equations : 

x = f(u, i;), y = <p(u, 0), z = t(u, v), 

where these functions are continuous together with their first 
derivatives, and not all the Jacobians 



d(u,vy d(u,v)' d(u,v) 

vanish. The element of arc is given by the formula : 

ds* = Edu* + 2Fdudv + Gdv\ 
where the coefficients arc easily computed, 



The kinetic energy has the value : 

T = % (Eu* + 2Fui> + 



Lagrange's Equations now become, since U = : 
(6) 



(Eu + Fit) - i (E u w 2 + 2F U uv + G u t- 2 ) = 0, 



(Fu + Gv) - - (E v u 2 + 2F v uv + G v v 2 ) = 0. 

On the other hand, the geodesies, in their capacity of being 
the shortest lines on the surface, are given as extremals of the 
integral A , 

= fVEu' 2 



L = / VEu' 2 + 2Fu'v' + Gv' 2 d\ 

*0 



* By a geodesic is meant a line of minimum length on a surface minimum, at 
least, if the points it connects are not too far apart ; cf. Advanced Calculus, p. 411. 



LAGRANGE'S EQUATIONS. VIRTUAL VELOCITIES 309 

in the Calculus of Variations (cf. the Author's Advanced Calculus, 
p. 411) by the equations : 

Eu' + Fv' E u u' 2 + 2F U u'v' + G u v' 2 

- = 



d Fu' + Gv' E v u'* + 2F V u'v' + G, v'* _ 

= u 



(7) 

d\ VEu'^'2Fu'v r + Gv' 2 2V'Eu' 2 + ^'u'i/^W 2 
The parameter X can be replaced by any other parameter, /u : 

M = /(A), 

provided that/(X) is continuous, together with its first derivative, 
and/'(X) 9* 0. In particular, then, the choice t = /z is a possible 
one. But then, because of the equation of energy, T = h, or : 



(8) (#w' 2 + 2*W + Gv'*) = h, u' = u, v' = *, 

i 

it follows that Equations (7) reduce to Equations (6). 

Since the velocity along the path is constant, the only force 
being normal to the path, t is proportional to 5. In fact, (8) 
says that 

mds * 



Thus the transformation of the parameter from X to t amounts 
in substance to a transformation to s; i.e. Equations (6) are 
virtually the intrinsic differential equations of the geodesic : 



(9), 



~ (Eu' + Fv') - (E. w' 2 + 2F U u'v' + G u v"*) = 
as 

J- (Fu f + Gv') - $ (E, w' 2 + 2F V u'v' + G, v' 2 ) = 
as 

. du . dv 

U* = -J-, V' = -7- 

rl n ' ft n 



EXERCISES 

1. Obtain the geodesies on a cylinder of revolution. Observe 
that, when the cylinder is rolled out on a plane, the geodesies 
must go over into straight lines. 

2. The same problem for a cone of revolution. 



310 



MECHANICS 



3. Show that the geodesies on an anchor ring, or torus, are 
given by the differential equations : 

d 2 . h 2 sin 6 



(10) 



a(b + acosfl) 3 



" 



where a and & > a are the constants of the anchor ring, and A is a 
constant of integration. 

4. Show that if, in the preceding question, initially 6 = ir/2, 



= or, 



= A then 



(ID 



a 2 (6 + a cos0) 2 a 2 



dt (b + a cos 0) 2 
6. Lemma. We have seen in 2 that, in the case of a single #, 



dx (Py dy 
dq dt 2 dq 



d^z 
dt 2 



dt dq dq 

It is important to recognize this equation as a purely analytic 
identity, irrespective of any physical meaning to be attached to 
T. It says that, if 

T = ~(x 2 + y 2 + z 2 ) 
and 

* = f(q, 0, y = v(<7, 0, ^ = ^(<7, 0, 

where these functions arc any functions subject merely to the 
ordinary requirements of continuity, then Equation (1) is true. 

We turn now to the general case of n particles, m with the 
coordinates (a?, yt,Zi) 9 i = 1, 2, , n. Let the position of 
the system be determined by m parameters, or generalized coordi- 
nates, ?!,, q m , and the time, t : 

*i = /ifoi, ' ' ', ?m, 

yi= <Pi(q ly -, ?m, 

2i = ti(qi, - , gm, 

where the functions /,-, (p, ^ t , are continuous together with their 
partial derivatives of the first two orders, and where the rank of 
the matrix a) is m : 



A) 



LAGRANGE'S EQUATIONS. VIRTUAL VELOCITIES 311 



a) 



dx l 
dq m 



dq l 



The kinetic energy, 



can be expressed in terms of g lt - , q m , q ly , q m , t, for 

with similar formulas for y iy z^ 

Our aim is to establish the general fundamental formula cor- 
responding to (1) : 



i \ 



-^~' - " 



r = 1, 



The independent variables in the partial differentiations are 
(<7i> ' " (7m, (7i> > qm, 0> and x^ y^ Zi are given by (3). We 
have : 



From (3) : 
Hence 



_ _ 
dq r 'dqr 



- etc. 



Differentiate with respect to ^ along a given curve : 
(A\ <L?L = V (tfxjdxj d^jjdyi d 2 Zj dz 

W *^ r V mi V"^ 2 0?r ^ 2 ^r ^ 2 07 

d dxi d^dy/i . d[ dzj\ 

2 ' 



312 



MECHANICS 



On the other hand, 

(5) I = 

Now, 

For, from (3), 



\ * dq r * dqr l dqr< 



^ 
dt 



while 



d 



dq r dt' 



dtdq r 



Similar relations hold for diji/dq r and dZi/dq r . On substituting 
these values in (5), it is seen that the last sum in (4) has precisely 
the value dT/dq r , and thus the relation I. is established. 

7. Lagrange's Equations in the General Case. Let a system 
of particles nti with the coordinates (xi, y^ Zi) be acted on by any 
forces whatever, X, F t , Zi. By Newton's Second Law of Motion 



(i) 



v 

= Xi 



Let the position of the system be determined, as in 6, by m 
coordinates q l9 , q m and t : 



A) 



where the functions /-, ^,-, 

derivatives of the first two orders, the matrix 



ifei, ' , <7 
(<7i, , ? w , 

i(^li ' ' ' i (7m, 

are continuous together with their 



dq l 



LAGRANGE'S EQUATIONS. VIRTUAL VELOCITIES 313 

being of rank m. Multiply the first of Equations (1) by 8xi/dq r , 
the second by dy t /dq r , the third by dzi/dq r , and add : 



/0 , v ( x * x < 

(2) 2, *< VdP" ft 






dx < 4. v ^< j. 7 ^A 

^ ^ ^' 

r = 1, , ra. 

The left-hand side has the value expressed by the Fundamental 
Equation I. of 6. Let the right-hand side be denoted by Q r : 

(3) " 

It thus appears that 

d dT 



These are known as Lagrange's Equations. 

We have deduced Lagrange's Equations from Newton's Second 
Law of Motion. They include Newton's Law as a particular case. 
For if we set 



t = 

then T 7 becomes : 



and Q 3 <, Q 3 <+i, Qa<+2 are now the components of the force which 
acts on m t -. Thus Newton's Equations result at once. 

8. Discussion of the Equations. Holonomic and Non- 
Holonomic Systems. We have before us the most general case. 
No restrictions have been made on the forces. These may, then, 
comprise dissipative forces, like those of friction or air resistance. 

On the other hand, there may be one or more equations of the 
form: 



(4) 

where the function F does not depend on the initial conditions. 



314 MECHANICS 

Moreover it may happen, whether there are relations of the 
form (4) or not, that the <?/s and their time derivatives are bound 
together by one or more equations : 



(5) $(?!, ' ,?m, % , ?m, = 0. 

An airplane, rising at a given angle, would be an example. 

The case which is most important in practice, is that in which 
<f> is linear in the q r : 

(6) AM + -- +A m q m + A = 0, 

where the A's are functions of (q lt , q m , C), independent of 
the initial conditions. 

It may happen that a relation of the form (6) is equivalent to 
one of the form (4). Thus if 

' ds dO 



this relation is equivalent to the equation : 

(8) s - ad = c, 

which is essentially of the form (4). 

If no relations (5) or (6) are present ; or if such relations (5) or 
(6) as may have entered in the formulation of the problem are 
all capable of being replaced by equations of the form (4), the 
system is said to be holonomic. Examples of non-holonomic systems 
are the Cart Wheels of 24 infra, and the Billiard Ball on the 
rough table, rolling and pivoting without slipping, p. 240 ; also the 
coin on the rough table, and the bicycle.* But when the Billiard 
Ball slips, p. 237, the system is holonomic, for the unknown reac- 
tion of the table can be computed explicitly, as the reader can 
easily verify, in terms of the velocity of the point of contact, 
and thus its components are expressed in terms of the time deriv- 
atives of the generalized coordinates. 

We are still leaving in abeyance the question of whether La- 
grange's Equations admit a unique solution. Our conditions are 
necessary for a solution of the mechanical problem, but not always 
sufficient. The study of sufficient conditions will be taken up in 
17 and in Appendix D. 

* Appell, Micaniqae rationelle, Vol. II, Chaps. XXI, XXII. 



LAGRANGE'S EQUATIONS. VIRTUAL VELOCITIES 315 

9. Continuation. The Forces. The question of holonomic or 
non-holonomic has to do with the left-hand side of Lagrange's 
Equations, i.e. with conditions on the q r , q r , t which do not involve 
the forces or contain the constants of the initial conditions. 

The forces appear on the right, and it is to these that we 
now turn our attention. It may happen that the total force 
Xi, Yij Zi can be decomposed into two forces : 

(9) x, = xi + xi Y< = Yi + 17, z t = z( + z; 

in such a manner that the X{, Y^ Z\ will be essentially simpler 
than the X, Yi, Z iy and that the X*, F*, Z* disappear altogether 
from Lagrange's Equations. For example, the X{, F{, Z\ may be 
expressible in terms of a force function : 

v , _ till v , _ d(J r/r _ dU 
Xi ~ ~ Yi " ' " 



where U is known explicitly in terms of X*, 2/, ,-, t. 

As regards the disappearance of the A7, Y*, Z* the problems 
discussed in 1-6 have afforded ample illustration. These 
were the so-called forces of constraint, and they did not appear in 
Lagrange's Equations. 

Returning now to the general case, we observe that it may 
happen that the X*, F*, Z* fulfil the condition : 



r 1, , m. When this is true, the Q r on the right of La- 
grange's Equations take on the simpler form : 



This case is important in practice because it enables us to get 
rid of some or all of the unknown forces of the problem arising 
from constraints ; cf . 1 5. But even when all of the latter forces 
cannot be eliminated in this way, their number can be reduced to 
a minimum ; and then the method of multipliers set forth in the 
next paragraph leads to the final elimination. 



316 



MECHANICS 



10. Conclusion. Lagrange's Multipliers. Consider a system, 
the motion of which is given by Lagrange's Equations : 

ddT_dT^ = Q 

It can happen that the Q r 's can be split in two : 

(14) Q r = Qr + &*, r = 1, - , m, 

in such a manner that the Q' are essentially simpler than the Q r 
known functions, for example whereas the Q* have the 
property that 

(15) Q*TT, H + Qiirm = 0, 

where ir lf , w m are any m numbers which satisfy the equations : 

(16) disTTi + + a ms Tr m = 0, s = 1, -,/*< m. 
Let the rank of the matrix 



(17) 



be u. 



a n 



a m i 



From Equations (13) it follows that 
d dT dT ~ 



no matter what numbers the TT, may be. If, in particular, the 
Q r and the jr, are subject to the condition expressed in (14), 
(15), and (16), then 



(18) 



d dT 



Multiply the /z equations (16) respectively by arbitrary num- 
bers, Xi, , X^, and subtract from (18) : 



Of the m numbers v lt 9 v m it is possible to choose some 
set of m p, arbitrarily, and then the rest are determined by 
(16). For definiteness, suppose 



LAGRANGE'S EQUATIONS. VIRTUAL VELOCITIES 317 

(20) 

Then ir^+i, ,ir m are arbitrary, and ir u , TT> are determined. 
Now let the Xj, , V be so chosen that 

(21) 



This is possible because the determinant of these /z linear equa- 
tions in X,, , X M is not zero. For these values of X Equa- 
tions (19) reduce to the following m ju equations : 



(22) 



The determination of the X's by (21) is independent of any 
choice of the TT/S. The numbers TJ>+I, , TT OT are wholly arbi- 
trary. Hence each coefficient in (22) must vanish. We have 
thus established the following 



THEOREM. When Q r can be written in the form: 



(23) 
w/ie 
(24) 



r = 1, 



(25) , a ls *-! + 

the rank of the matrix 

(26) 



+ a ma 7r m = 0, 



= 1, 



a m \ 



Ctl/x ' ' ' 



iwgf /z, </ien i< zs possible to find p numbers \ 19 , X^ swcA 



(27) 



dT 



numbers are determined by & of the Equations (27), and the 
values thus obtained are then substituted in the remaining m p 
equations. 



318 MECHANICS 

Applications of this theorem occur in practice in a variety of 
problems in which the q r , q r , and t are connected by relations of 
the form (6), 7 : 

(28) ai,^ + + a m qm + a, = 0, = 1, ,/*, 

where the a r ,, a, depend on the q r and , but not on the ini- 
tial conditions. As a matter of fact, in a number of such 
cases the coefficients a ra in (28) do lead to a system of equations 
(16) which control a set of numbers TT^ , w m for which an 
analysis (14) of Q r with the resulting relation (15) is possible. 

In other problems, however, the a rs of equations (16) have noth- 
ing to do with any such equations as (28), if indeed the latter 
exist, but may even themselves depend on q r , as well as q r and t. 
For a complete discussion cf . Appendix D. 

We turn now to a direct determination of the Q r from purely 
mechanical considerations. 

11. Virtual Velocities and Virtual Work. Let a system of 
particles ra with the coordinates (x %1 ?/ t , z t ) be given (i 1, 
, ft). Let dxi, dyt, dzi be any 3n numbers, and let m be 
carried to the point (xi + 8x l , yi + fyi, Zi + dZi). Then tha 
system is said to experience a virtual displacement (5xi, tyi, dZifl 
the word " virtual" expressing the fact that the actual system 
may not be capable of such a displacement, even approximately. 
Thus a particle constrained to move on a curve or a surface would 
in general be taken off its constraint, and not lie even in the tan- 
gent line or plane. 

If forces (Xi, Y^ Z$ act on the system, the quantity 

(1) W* = J (X, dxi + Yi d yi + Zi dzi) 

t = i 

is defined as the virtual work due to the virtual displacement. 

It is convenient in many applications to restrict the virtual 
displacements admitted to consideration by linear homogene- 
ous equations between the 5x t -, 6?/ t , 5zi. Consider, in particular, 
a system of particles whose coordinates are given by Equations 
A), 7: 

^ = fi(qi, - - , q m , t) 



A ) 



, 
*, 



LAGRANGE'S EQUATIONS. VIRTUAL VELOCITIES 319 

where the rank of the matrix 



a) 



is m. Let 



(2) 



fat t dx l 

09i dq m 

^ dZ n 

dq l dq m 



where dq } , , 3q m are m arbitrary quantities. If m < 3n, the 
toi, 8y i} dzi are subject to one or more linear homogeneous equa- 
tions. Thus only a limited number of them can now be chosen 
arbitrarily, the rest being then determined. 

Consider the actual displacement (Ax t -, A?/*, Az) which the 
system experiences in time At as it describes its natural path. 
It is : 

AXt = fi (q l + Ag,, , q m + Ag m , t + At) / (q ly , q m , t) 
(3) A?/t = <pi (q l + At/!, , q m + A^ m , t + A^) pi (q lf , g m , ^) 

Since the 5# r are arbitrary, it is possible to choose them equal to 
the Aq r , or dq r = Aq r . It does not follow, however, that the cor- 
responding tot, diji, dzi will differ from Ax i} Ay iy Az by infinites- 
imals of higher order with respect to A. This will, in fact, be 
the case if the functions / t -, <p t , \f/i do not contain the time, i.e. 
if dfi/dt = 0, etc. But otherwise in general not. 
The virtual work has the value : 



(4) 



, 



where all m of the numbers 8q r are arbitrary. If, in particular, 
the forces can be broken up as in (9) 9 : 

(5) Xi = XI + XI Ft = Y( + F?, Zt = Z\ + Zt, 



320 MECHANICS 

so that (11) holds: 

(6) jjj(ir* +17* + * 

r = 1, , m, then (4) takes on the simpler form : 



(7) r,- 

In either case, 
(8) W 5 = Q.dq, + ...+Q m 8q m . 

Consider the actual displacement (Ax, Ayi, AZi) of the system 
in time At as it describes its natural path. If /,-, ^? t -, \f/i do not 
contain t, the virtual work W s will differ from the actual work, 
ATT, by an infinitesimal of higher order than A; otherwise, this 
will not in general be the case. 

12. Computation of Q r . In Equation (8), 11 the dq r are 
m arbitrary numbers. We may, then, set dq k 0, k ^ r; 
5q r 7* 0, and compute the corresponding value of W 6 . We shall 
then have : 



Consider, for example, a particle that is constrained to lie 

on a moving surface. Its coordinates are subject to the condi- 
tions : 
(10) x = f(q ly q 2 , 0, y = <p(qi, q 0, 2 = iKfc, q* t). 



A virtual displacement means that we fix our attention on an 
arbitrary instant of time, t, and consider the surface represented 
by (10) for this value of t. Next, consider a point (x, y, z) of 
this surface. Then a virtual displacement (&r, dy, dz) of this 
point means an arbitrary displacement in the tangent plane to 
the surface at the point in question. In particular, if we set 
dq 2 = and take dq 1 ^ 0, then the virtual displacement takes 
place along the tangent to that curve in the surface whose coor- 
dinates are represented by (10) when </ 2 and t are held fast. 

Now, the natural path of the particle under the forces that 
act does not in general lie in the surface just considered, nor is 
it tangent to the surface. If the surface is smooth, the reaction 
on the particle will be normal to the surface, and so the virtual 



LAGRANGE'S EQUATIONS. VIRTUAL VELOCITIES 321 

work W s due to the reaction will be 0. But the actual work 
done by the reaction in A seconds along the natural path will 
in general be an infinitesimal of the same order as At. 

It is now easy to see how to compute Q l and Q z m case the 
surface is smooth. The virtual work of the reaction of the surface 
is nil, and so we need consider only the other forces. The virtual 
displacement takes place in the tangent plane to the surface, 
and we can compute directly the virtual work corresponding 
to the successive virtual displacements given by 8q l ^ 0, 8q 2 = 
and 5ft = 0, 8q z ^ ; cf. further 16 infra. 

13. Virtual Velocities, an Aid in the Choice of the ir r . In 
the general theorem of 10 there was no indication as to how 
the 7r r may bo chosen. In certain cases which arise in practice, 
the motion being subject to Lagrange's Equations : 

/ d 3T dT 



it happens that there are geometric or kinematical relations 
between the q r 's of the form (28), 10 : 

(2) a li(f ft + ' ' + dmsqm + CL 8 = 0, 8 = 1, -,/*< 1, 



where the a r8 , a 8 are known functions of q lt , q m , t,* which 
do not depend on the initial conditions, and where the rank of 
the matrix 

a n 
(3) 



IS fJL. 

If, now, the possible virtual displacements corresponding to 
an arbitrary choice of 5ft, , 8q m are so restricted that 

(4) a ls 8qi + - - + a m8 8q m = 0, 5 = 1, , /*, 

it turns out that the virtual work of certain forces ("forces of 
constraint ") will vanish. Hence by identifying these "forces 
of constraint " with the Q* and setting 8q r = 7r r , the hypotheses 
of that theorem arc fulfilled. 

* It may happen that some or all of these equations may be integrated in the 
form: F (qi, -, </ m , t) = 0, where F does not depend on the initial conditions; 
but it is not important to distinguish this case. 



322 MECHANICS 

Example. Consider the disc of Chapter VI, 24 as free to 
roll without slipping on a rough horizontal plane which is moving 
in its own plane according to any given law ; for example, rotat- 
ing about a fixed point with constant velocity. The force which 
the plane exerts on the disc at the point of contact will do work 
on the disc. But the virtual work of this force, when the virtual 
displacement is restricted as above, is nil. Thus we are led to 
a suitable set of multipliers 7r r , namely, the 5q r thus restricted. 

14. On the Number m of the q r . For a system of particles 
the q r 's, as has already been pointed out, can always be identified 
with the coordinates : 

Here, m = 3w, and Lagrange's Equations become identical with 
Newton's Equations. 

In 'theory, then, there is no difference between the two systems. 
In practice, Lagrange's Equations provide in many cases an 
elimination of forces in which we arc not interested. 

Consider a ladder sliding down a wall. If the wall and floor 
are smooth, we may take m = 1, q = 0, and all the forces in 
which we are not interested will be eliminated. 
s Here, 

(2) x = a cos 0, y = a sin 0. 

MgeM K Hence 
FIG. 144 ( 3 ) r = ^(02 + 1)0. 

Lagrange's Equation becomes : 

where 

U = Mg a sin 0. 

Thus we find as the equation governing the motion : 

M (a 2 + A; 2 ) -^ = - Mga cos 

or 

fK\ d?0 ag 




LAGRANGE'S EQUATIONS. VIRTUAL VELOCITIES 323 

In this example, the maximum of elimination has been at- 
tained at one blow. If we think of the ladder as made up of a 
huge number of particles connected by weightless rods, the forces 
in the rods have been eliminated, and also the forces exerted by 
the floor and the wall. 

Suppose, however, that the floor and the wall 
are rough. We can still write down a single 
Lagrangean equation, 

the left-hand side being as before. But now 

W 

(7) Q = _J = - Mga cos + 2a cos Op,S + 2a sin R. 

dq 

We have not equations enough to solve the problem. 
The difficulty can be met by taking m = 3 and setting 

(8) 0i = x, 02 = 27, 03 = 0- 
T is given by (1). And now 

Q! = S - M#, Q 2 = R + S - Mg, 




(9) 

1 = a(sin + cos 0) S + a(/i sin - cos 6) R. 

Lagrange ; s three equations become : 



(10) 



= a ( s in + n cos 0) S + aO sin - cos 0) 



The first two of these are the equations of motion of the centre 
of gravity ; the third, the equation of moments about the centre 
of gravity. 

What Lagrange's method here has done, is first to eliminate 
the internal forces between the particles, just as we did in Chapter 
IV, 1, when we proved the theorem about the motion of the 
centre of gravity; and similarly, when we proved the theorem 
of moments, Chapter IV, 3 and 9. 



324 MECHANICS 

Let 

Qr = + Qf, 

where 

Qr~s-MB, Q; = /Z + /*S, 

Q* = a(sin + /x cos 0) S + a(p, sin - cos 6) R. 
We wish to find three multipliers, TT^ ?r 2 , 7r 3 , such that 
(11) Ql^ + Q*T 2 + Q,*T, = 0. 

This can easily be done algebraically, with the result that 
TT I + /i7T 2 + a(sin 6 + /x cos 0) 7r 3 = 



(12) , 

+ 7r 2 + (M sin cos 0) 7r 3 = 

a solution of these equations being : 

TJ = sin (0 + 2X), ?r 2 = cos (0 + 2X), 7r 3 = I/a. 

But a mechanical derivation is easy, too. Consider the result- 
ant of the forces R and p,R. Draw a perpendicular to it through 
the lower end of the rod, and displace this end along this line. 
Do the same thing at the upper end of the rod, and displace the 
upper end along this line. The result is, that 

f Sq l =-asin (9 + 2\) 8q, 
' lo) 1 

I dq 2 = a cos (6 + 2X) S# 3 

Corresponding to such a displacement the virtual work of the 
"constraints" must vanish. And now it is merely a question of 
trigonometry to show that our expectation is fulfilled : 

(14) Qj>i + Ql fy, + ,*?, = 0. 

Equation (11) corresponds to Equation (15) of 10, and Equa- 
tions (12) are the Equations (16) of that paragraph. But Equa- 
tions (13), though corresponding to Equations (4), 13, do not 
have their origin in Equations (2), 13. The latter would arise 
from differentiating (2). 

Returning now to Equations (10), we see that the unknown 
reactions R and S are eliminated by (14), where 5q lf 8q. 2 , 8q s sat- 
isfy (13). Hence 

(15) Jflfift + (M + Mg) dq, + Mk*0dq z = 0, 
or 

(16) - MX a sin (0 + 2X) + (My + Mg) a cos (0 + 2X) 

+ Mk* '6 = 0. 



LAGRANGE'S EQUATIONS. VIRTUAL VELOCITIES 325 

This equation, combined with Equations (2), leads at once 
to the solution of the problem : 

(17) (/c 2 + a 2 cos 2X) ~~ + a 2 sin 2X ^~ + ag cos (0 + 2X) = 0. 

15. Forces of Constraint. A definition of "forces of con- 
straint" from the point of view of physics, which shall be both 
accurate and comprehensive, has, so far as the author knows, 
never been given. They would be included in such forces as 
the X*, *, Z* of 9, which disappear from the Q r ; I.e., Equa- 
tion (11). Arid still again, the Q* of 10 arise from unknown 
forces and are eliminated by the method of multipliers. 

Perhaps these two cases are comprehensive in Rational Me- 
chanics. Are there problems in this science not included here? 
If not, the asterisk forces could be defined as the forces of con- 
straint ; cf . Appendix D. 

16. Euler's Equations, Deduced from Lagrange's Equations. 

When a rigid body rotates about a fixed point, the kinetic energy is 

(1) T = i(4p 2 + #? 2 + O 2 ). 

Let p, q, r be expressed in terms of Euler's angles, Chapter VI, 
15: 

p = 6 sin (p \}/ sin cos <p 

(2) q 6 cos <p + \l/ sin Q sin <p 
r <j> -{- \l/ cos 

The second of Lagrange's Equations is readily computed : 

dT A dp . ,, dq . dr 
= Ap~ + Bq~~ + CV = Cr; 



v<P O(D V(D (/<p 

TT- = 8 cos <p + ^ sin 6 sin <p = g, 

= 6 sin v> -\- $ sin cos ^> = p, 
Hence 



326 



MECHANICS 



To compute <$>, observe that, no matter what forces may act, 
they can be replaced by a force at and a couple. The latter 
can be realized by means of three forces : 



o 

ii) 
Hi) 



a force L y acting at the point * r = 
" Ma " " r = 



T = a. 



A virtual displacement 80 = 0, 5<p ^ 0, d\l/ = gives as the 
virtual work 

N5<p 

and this is equal to &8<p. Hence <t> = N and we have : 
Cj|- (A -B)pq = N. 

This is the third of Euler's Dynamical Equations. The other 
two follow from this one by symmetry, and are obtained by 
advancing the letters cyclically. 

EXERCISE 

Obtain the six equations of motion of a rigid body by means of 
Lagrange's Equations. 

17. Solution of Lagrange's Equations. We have seen in 
10 that if the Q r satisfy the conditions of the Theorem of that 
paragraph, then 



(i) 

where the matrix : 
(2) 



- 

dt dq r dq r 



y* ^ 
= Qr + 2) a r8 \ 9 , r = 1, , m, 



is of rank ju < m. In the cases which arise most frequently in 
practice, there are n equations of the form : 



* By the " point r " is meant the terminal point of the vector r when the initial 
point is at 0. 



LAGRANGE'S EQUATIONS. VIRTUAL VELOCITIES 327 

(3) a,i s qi + - + a ms q m = a a , s = 1, , ju, 

where the a's are functions of g lt , q m , t. 

The kinetic energy T is a positive definite quadratic form in 
the q l9 , q m , but not necessarily homogeneous : 

T = T 2 + T,+ T , 
where 



and T 19 T are homogeneous of degree 1 or in the q r , or van- 
ish identically. The coefficients are functions of q lf - - , q m , t. 
The form T 2 , or 

(4) 2 </*<** 



*,./ 



is a positive definite homogeneous quadratic form. For T can be 
written in the form : 



/tu, , ju w , (7 are functions of #i, -, ^ m , t. 
Finally, let Q' r be a known function of q r , q r , t. 

THEOREM. The m + /* Equations: 

d dT 8T / A 



i H ---- + o.g = a., s = 1, , /z, 
determine uniquely the m + p, functions (ft, , </, X x , , X M . 
Proo/. The first m of these equations have the form : 

(5) A ir qi + + A mr q m a rl Xj a r/A X M = B r , 

r = 1, , m, where r is a function of the </,., q r , and . The 
remaining /* equations give, on differentiating : 

(6) ai,qi -\ ---- + a m sqm = C a , s = 1, , /*, 



where C. is likewise a function of the g r , q r , and <. Thus we have 
m + M linear equations in the m + n unknowns: q lt , # m , 
Xj, , X^. Their determinant : 



328 



MECHANICS 



_ 

"" an aii 

Oi,A Om M 

does not vanish. For otherwise the m + n linear homogeneous 
equations : 

u ti + + AmiZm + an*?! + + ai^ = 

lmti + * ' + Ammtm + Oml^ + ' ' ' + Omplfc = 

= 

= 

would admit a solution (, - , w , 77^ , T/ M ) not the identity. 
Moreover, not all the fi, , m in this solution could vanish ; 
for then we should have : 



+ 



+ 



= 0. 



But the rank of the matrix of these equations, namely the matrix 
(2), is /x. Hence all the i) l9 , ^ of the solution vanish a 
contradiction. 

Next, multiply the r-th equation (8) by r , r = 1, , m, and 
add. The terms in i^, , 77^ drop out because of the last p. of 
the equations (8), and so there results the equation : 



where not all the j, , m are 0. This is impossible, since (4) 
is a positive definite quadratic form. 

Equations (5) and (6) admit, therefore, a solution : 



(9) 



0, 





, m ; 



LAGRANGE'S EQUATIONS. VIRTUAL VELOCITIES 329 

Assuming for definiteness that the determinant 

a n <v 



I/*'** Uft.fi. 

wo see that the first m of the Equations (9) admit the integral 
given by (3), or : 



where, in particular, /, is linear in <fo+i, , q m - This is a par- 
ticular integral which is independent of the initial conditions of 
the mechanical problem. Let 

(11) q a = K a , a = + 1, - , m. 

The system of m differential equations (9) is now seen to be equiv- 
alent, under the restrictions of the dynamical problem, to the 
system : 

dq 8 f , j\ 1 

' ' ' ' ' * - - ' 



(12) 

d Ka 



, Km, 0, tt = /* + 1, 



Here is a system of 2m p differential equations of the first order 
for determining the 2m M unknown functions q r , K a . Their 
solution yields the m desired functions, q lt - - - , q m . The X 8 are 
now uniquely determined as functions of t and the initial condi- 
tions. As regards the freedom of the initial conditions, on which 
of course the determination of the constants of integration depends, 
the initial values </ r , g r of q r , q r are restricted by the equation 

fl\sf]\ H I * * * I drnsqm ~ $.s- 

It is important here, as in so many problems of the kind dis- 
cussed in this chapter, to distinguish between constants that are 
connected with the choice of coordinates and constants that arise 
from the initial conditions of the mechanical problem. Thus in the 
problem of ('hap. IV, 13, p. 141, Fig. 84, s might equally well 
have been measured from a different level, and then the relation 
would have been : 

s = ad + c. 



330 



MECHANICS 



18. Equilibrium. Let a dynamical system be given, with n 
particles m,, the motion being subject to Newton's Law : 



(1) 



The forces are said to be in equilibrium if 



Z it 



1, 



n. 



(2) 



= 0, Y t = 0, 



0, 



A necessary and sufficient condition for equilibrium is, that 



(3) 



= 0, 



= 0, 



= 0. 



We are not interested in the general case, which, in accord with 
the definition just given, relates to a single instant of time, the 
forces not in general being in equilibrium at any other instant. 
We have concern rather with a permanent state of rest of a system 
capable of certain motions which are subject to geometric condi- 
tions. We are thinking primarily of such problems in the statics 
of particles and rigid bodies as were studied in Chapters I and II ; 
but also of more general problems, like the following : A uni- 
form circular disc has a particle attached to its rim. The disc 
rests on a smooth ellipsoid and a rough table which contains 
two axes of the ellipsoid. Find the positions of equilibrium. 

More precisely, the system shall be capable of assuming the 
positions defined by the equations : 



(4) 



= fi(q\, ,?*) 



where the functions /, ^, \f/i do not depend on t, and where the 
rank of the matrix 



(5) 



s ra. 

Observe that this last requirement does not imply that m has 
the least value for which the x iy y^ Zi can be represented by equa- 
tions of the form (4), satisfying the above requirements. It is 



LAGRANGE'S EQUATIONS. VIRTUAL VELOCITIES 331 

still possible that the q 19 , q m may be connected by relations 
of the form : 

(6) Ft (ft, , q m ) = 0, j = 1, , p < m. 

On the other hand it does imply that if the x^ y iy 2, all vanish, 
then this is true of the q r , and conversely; and if, furthermore, 
both the ij #, z, and the x iy #, z all vanish, then this is true 
of the q r and the q r , and conversely. 

The motion of the system is, first of all, subject to the equa- 
tions : 

(7) [71, = Q r , r = 1, , M < m, 

where by definition 

\T\ =<L2L-VL. 

1 lr dt dq r dq r 
To these may be added further equations : 

(8) a la qi + + a m *q m = 0, a = 1, ,/*< m, 
where the rank of the matrix 



(9) 



is (1. It is possible that some or all of these equations can be 
expressed in the form (6), but this is unimportant. 

A first necessary and sufficient condition for equilibrium is that 

(10) Q r = 0, r = 1, - - - , m. 

For, a necessary and sufficient condition for the vanishing of the 
left-hand side of (7) for ft = 0, ,&, = is that ft = 0, 
- , q m = 0. 

If there are relations of the form (8), it may happen that the 
Q r can be split up as follows : 

(11) Qr = Qr + Q?> 

where 

(12) Q*ft + + Q* m *qm = 0, 

provided the dq r are so chosen that 

(13) 01,30! + + Om^qm = 0, s = 1, , /*. 



332 MECHANICS 

Under these circumstances a necessary and sufficient condi- 
tion for equilibrium is that 

(14) <?>/! + - +Q' m dq m = 0, 

provided the 8q r satisfy (13). 

That the condition is necessary appears from the fact that 
(10) is true, and hence 

(15) (Q[ + <#) & + + (<& + Qi) ?* = 

for all values of the dq r . If the 5q r satisfy (13), it follows that 
(12) is true, and (14) now follows. 

Suppose conversely that (12) and (14) hold when the 8q r are 
subject to (13). Then the system is in equilibrium. Suppose 
the statement false. From (12) and (14) it follows that (15) holds, 
provided (13) is true, and hence from (7) it follows that 

(16) i)[r]r5<y r = 0, 

T~.\ 

provided (13) holds. Lot 

(17) q r = c r , r = 1, , m, 
initially. Then not all the c r are 0. Now, 

(18) dq r = c r , r = 1, , m, 

is a system of values satisfying (13). For, on differentiating (8) 
with respect to t and then setting t = / , q r = 0, these relations 
follow, namely : 

0>lsC\ + ' ' ' + OmsCm = 0, S = 1, , (JL. 

Consequently (16) holds for those values of c r . Now, 

(19) ' T = ^A^q a q ft . 

a, ft 

Hence 

f)T 

= Ai r (ji + ' ' ' + A m rqmj 
v(]r 

d BT .... , A .. . . . ,. . , 

^ -QT = Air q\ + - - + A mr q m + terms in (q l9 - , q m ), 

and so initially 

m m 

^ [T] r dq r = ^ MirCj H + A mr c n )c r = ^ A a pc a c ft . 

-! r=l a,/3 



LAGRANGE'S EQUATIONS. VIRTUAL VELOCITIES 333 

But hero is a contradiction, since (19), being a positive definite 
quadratic form, can vanish only when all the arguments are 0. 
We can state the result as a 

THEOREM. A necessary and sufficient condition that a dynamical 
system, the motion of which is governed by the equations : 

_rf d_T __ 8T 

(20) dt'dq r Wr~ V " r - 1 '"-> m; 

i7i + + Om. (7m = 0, = 1, ,/*< m, 
where the rank of the matrix of these last p, equations is /*, be in 
equilibrium and at rest, is that q r = 0, r = 1, , m, and that 

(21) Qiffi + +Qmdq m = 0, 
where. 5q } , - - , dq m are subject to the condition: 

(22) a\8qi + + a m5 <$tf w = 0, = 1, -,/*. 

7 T is a homogeneous positive definite quadratic form in 



//, in particular, 

(23) Q r = Qr + Qr*, f = 1, , m, 

and ?/ # is known that 

(24) Q*fy, + + Q* n dq m = 0, 

where dq l9 , 5g m are subject to (22), ttew (21) can 6e replaced by 

(25) QlSft + - + Q' m dq m = 0. 

19. Small Oscillations. Two equal masses are knotted to a 
string, one end of which is made fast to a peg at 0. Determine 
the motion in the case of small vibrations. Here, 

T = ^ (202 + ^2 + 2 ^ cos fc, - 6 )), 

U = mga(2 cos + cos <p). 

Since 6, d, <p, <p arc small, these functions can be re- 
placed by the approximations : 

. 9X FIG. 146 



const. 




U = - mga(Q* + ^) + 



334 MECHANICS 

Equations (1) arc typical for an important class of problems 
in small oscillations of a system about a position of stable equi- 
librium, the applied forces being derived from a force function, 
(7. Let T and U both be independent of t\ let q r = for 
r = 1, , m, be the position of equilibrium, and let T, U be re- 
placed by their approximate values when q r , q r are all small. Then 



(2) T = V dra qr<ls 

r.s 



r, s = 1, - , ra, where the coefficients o r , = a ar , b r , = b, r are 
constants and each of the quadratic forms is definite. 
Lagrange's Equations now take the form : 

(3) Orltfi + ' ' ' + Cl rm q m = ~ (&rl<7l + + &rm?m), 

r = 1, - - - , m. 

*To integrate these equations, it is convenient to introduce new 
variables as follows. It is a theorem of algebra * that by means 
of a suitable linear transformation with constant coefficients : 

(4) q r = riq( + + Mmrf,, r = 1, - , ro, 

the quadratic forms (2) can each be reduced to a sum of squares : 
T = q(* + + q' m \ 
U = - n t 2 ft' 2 - - - - n m 2 ^ 2 . 
Lagrange's Equations now become : 

g $-V* r-l,...,. 

Their integrals take the form : 

(7) q' r = C r cos (n r t + 7r), r = 1, , m. 

Returning to the original variables q r , we find as the general 
solution of Equations (3) the following : 



(8) q r = CiMri cos (nj + TI) + + C m firm cos (n m t + 7m), 

r = 1, - , m, 
where the C r , y r are the 2m constants of integration. 

* Bocher, Higher Algebra, Chap. 13. 



LAGRANGE'S EQUATIONS. VIRTUAL VELOCITIES 335 

In this result, complete as it is in theory, there appear, how- 
ever, the coefficients /* r , of the linear transformation (4). These 
can be determined by the following consideration. 

Let C r = in (8) when r 9* s; and let C 8 = 1. Thus we have 
a special solution : 

(9) q? = \ r cos (nt + 7), 

where X r = /ir and n = n a , 7 = y 8 . Substitute q? in (3) : 

(10) (bn - n*a rl ) Xi H ----- h (b m - n 2 a rm ) \ m = 0, 

r = 1, - - , m. 

A necessary condition that (9) be a solution is, that the m linear 
Equations (10) admit a solution in which the X/s are not all 0. 
Hence the determinant of these equations must vanish : 



(ii) 



n 2 a n 



=o. 

6mm ~ n 2 a 



If the n r 2 are all distinct, they form precisely the m roots of 
this equation in n 2 . Moreover, each n? leads to a unique deter- 
mination of the ratios of the X's through the m Equations (10), 
and our problem is solved. 

It may happen that k of the roots n 2 of (11) coincide. In that 
case, k of the X's can be chosen arbitrarily, and so we still have k 
linearly independent solutions (9) corresponding to such a root 
n 2 . More precisely, let n 2 be a multiple root of order fcj ; n 2 2 , 
a multiple root of order fc 2 ; etc. Let n 2 be set = n^ in Equa- 
tions (10). Then, of the unknown \ lt , X m , it is possible to 
choose a certain set of ^ arbitrarily, and then the rest will be 
uniquely determined. Let all but one of these A^ X's be set 
= 1. Thus we get ^ sets of (X x , - - , X w ), and each set gives a 
solution of Equations (3). Moreover these solutions are obvi- 
ously linearly independent. Proceeding to n 2 2 we determine 
in the same manner fc 2 further sets of (X n . , X m ), each set giv- 
ing a solution of (3) ; these solutions are likewise linearly inde- 
pendent of one another and also of the earlier solutions. And 
so on, to the end. Thus in all cases the roots of (11) lead to m 
linearly independent solutions (9). 

The variables q' r are known as the normal coordinates of the 
problem. Each is uniquely determined, save as to a factor of 



336 MECHANICS 

proportionality, when the roots of (11) are distinct. But in 
the case of equal roots, an infinite number of different choices 
are possible. 

EXERCISE 

Carry through the example given at the beginning of the para- 
graph. 

Ans. Two sets of linearly independent solutions are the 

following : 
f 0j = cos fat + 7j), f 2 = cos fat + 7 2 ) ; 

i ^ = A/2 cos fat + 7i), I 02 = ~ ^ 2 cos fat + 7 2 ), 

where 

n* = (2 - V2) 2 n 2 2 = (2 + \/2) ? - 

Cv C* 

The general solution is : 

= <?! cos (n^ + TJ) + C 2 cos fat + 7 2 ), 

tf? = C^A/2 cos (n^ + TI) - C 2 V2 cos fat + 7 2 ). 

EXERCISES ON CHAPTER X 

1. A smooth wedge rests on a table. A block is placed on 
the wedge, and the system is released from rest. Determine 
the motion. 

2. Two billiard balls are placed one on top of the other, on 
a rough table, and released from rest, slightly displaced from the 
position of equilibrium. Determine the motion. 

3. A uniform rod is pivoted at one end, and is acted on by 
gravity. Will it move like a spherical pendulum ? 

4. A uniform rod of length 2a and mass 3m can turn freely 
about its mid-point. A mass m is attached to one end of the 
rod. If the rod is_rotating about a vertical axis with an angular 
velocity of \/2ng/a, and so released, show that the heavy end 
will dip till the rod makes an angle of cos~ 1 (Vn 2 + 1 ri) with 
the vertical, and then rise again to the horizontal. 

5. Obtain the equations of the top from Lagrange's Equations. 

6. Determine the motion of a top whose peg, considered as 
a point, slides on a smooth horizontal plane. 

7. The same question when the size of the peg is taken into 
account. 



LAGRANGE'S EQUATIONS. VIRTUAL VELOCITIES 337 

8. The ladder of p. 322, the initial position being oblique 
to the line of intersection of the wall and the floor.* 

9. Two equal rods are hinged at their ends and project 
over a smooth horizontal plane. Determine the motion. 

SUGGESTION. Take as coordinates (1) the x, y of the centre 
of gravity ; (2) the inclination 6 of the line through the centre of 
gravity and the hinge ; (3) the angle a between this line and either 
of the rods. 

Two of Lagrange's Equations control the motion of the centre 
of gravity. A third expresses the fact that the total moment 
of momentum with respect to the centre of gravity, is constant. 
And fourthly there is the equation of energy, f 

10. A rough table is rotating about a vertical axis. Study 
the motion of a billiard ball on the table, assuming that there is 
no slipping. 

11. The same problem with slipping. 

12. Work the problem of 19, p. 333, when the particles are 
not required to move in a vertical plane. 

13. Two equal uniform rods arc hinged at one of their ends, 
and the other end of one rod is pivoted. Find the motion for 
small oscillations in a vertical plane. 

14. The same problem when the rods are not restricted to 
lying in a plane. 

16. A uniform rod is supported by two strings of equal length, 
attached to its ends, their other ends being made fast at two 
points on the same level, whose distance apart is equal to the 
length of the rod. A smooth vertical wire passes through a 
small hole at the middle of the rod and bisects the line joining 
the fixed points. Determine the motion. 

16. If in the preceding question the wire is absent, study the 
small oscillations of the rod about the position of equilibrium. 

17. A bead can slide on a circular wire, no external forces 
acting. Determine the motion in two and in three dimensions. 
Begin with the case of no friction. 

* Routh, Elementary Rigid Dynamics, p. 329. 

t Appell, Mtcanique rationelle, vol. ii, chap. 24, 446. Many other problems 
of the present kind are found in this chapter. 



CHAPTER XI 
HAMILTON'S CANONICAL EQUATIONS 

1. The Problem. The problem of this chapter is the deduc- 
tion of Hamilton's Canonical Equations : 

dqr_m dpr__W i ... 

dt " dp r ' dt dq r ' ' ' ' 

from Lagrange's Equations : 

d dL dL n t 

:r; Q~ -- ^"~ = 0, r = 1, , m. 

cftd</ r dq r 

The transition is purely analytical, involving no physical con- 
cepts whatever, and for that reason it is well to set the theorem 
and proof apart in a separate chapter. 

The problem can be stated as follows. We start out with a 
Lagrangean System. Such a system is defined as a material 
system which can be located by means of m generalized coordi- 
nates q ly , q m and whose motion is determined by Lagrange's 
Equations. If we set q r = K r , these go over into the 2m equa- 
tions : 

A) 

d ML _ 

dt dK r dq r 
r = 1, < , m, where 

(1) L = L(q l9 ' , tfm, *i, ' , Km, = i(0r, *r, 

is a function of the 2m + 1 independent variables #/., * r , <. 

The function L is called the Lagrangean Function. In case 
there is a work function, 



L is given by the equation : 

(2) L = T + U, 

338 



HAMILTON'S CANONICAL EQUATIONS 339 

where K T = q r and 

T = T(q r , ? r , 

is the kinetic energy. In any case, the Hessian Determinant, 

the Jacobian : 

/\ d(L 1? - , L m ) 

(6) 0(*i,---,O' 

where 



shall not vanish. 

The (2m + l)-dimensional space S 2m +i of the variables (q r , * r , t) 
shall be transformed on the (2m + l)-dimensional space R 2m +i 
of the variables (q r , p r , t) by means of the transformation : 

/ M \ 8L t 

(4) Pr = ^-, r = 1, , m, 

the f/ r going over individually into themselves. The system of 
2m differential equations of the first order in the 2m dependent 
variables q r , K r , namely, Equations A), thereby goes over into 
a system of 2m like equations in the 2m dependent variables 
q r , p r . These last equations are the following: 

fr . dq r 811 dp r 8H - 

(5) -*=& -*=-*? r - 1 '-"-^ 
where II = H (q r , p r , t) is defined by the equation : 

(6) H = I) prKr ~ L, 

r=l 

the K r being functions of (q r , p r , defined by (4). 

This is the theorem which is the subject of this chapter and to 
the proof of which we now turn. The converse is true under 
suitable restrictions. 

2. A General Theorem. Let F(x l9 , x n ) be any function, 
continuous together with its derivatives of the first two orders, 
and such that its Hessian Determinant, the Jacobian : 

<" 



Let a transformation, T, be defined by the equations : 
T: r - r 



340 MECHANICS 

Let G (y lt , y n ) be defined by the relation : 

(2) G( yi , , j/n) = J x r y r - F(x l> -,x m ) > 

r=l 

where x l9 , x n are the functions of y lt , y n defined by 
1 . Then 



(3) x r -%, r- !,...,. 

For, differentiate (2), regarded as an identity in the independent 
variables y lt , y n : 

dx s 



The right-hand side, by the equation^ defining T, reduces to x r , 
and the proof is complete. Furthermore, 



For, on performing first the transformation T, then the transfor- 
mation T~~ l j the result is the identical transformation. Hence 



d(x u - - , x n ) d(y l9 , y n ) ' 
or: 

, G.) 1 



3(*i, , *n) 
In particular, then, 
/r v d(Gi. , G n ) r$(ri, , /n)"T~ 

f^i r= I I 

These results may be stated in the following theorem. 

THEOREM I. Let F(x ly , x n ) be a function satisfying the 
condition: 



Perform the transformation : 

dF 

T 11 r = 1 w 

^ . 2/r - , r 1, , n. 



HAMILTON'S CANONICAL EQUATIONS 341 

Let G(y lt , y n ) be defined by the equation: 

n 

(6) G(y ly , y) = 5) x r y r - F(x l9 , x n ), 

r=l 

where x r is determined as a function of (y lt , y n ) by the inverse, 
T~ l , of T. Then the inverse of T is represented as follows : 

T~ l x - r = 1 n 

1 . x r - ^, r l, , n. 

Moreover, 

d(Gi, ' ' ' > Gn) , Q 

^(2/1, -,2/n) 

In particular, 



The identical relation can be written in the symmetric form : 
(7) F(x lt ,x n ) 



r-1 

where 

3F dG 



and the Hessian Determinants of F, G are ^ 0. 

We now proceed to a second theorem, which is of importance 
in the applications of the results of this chapter in mechanics. 

THEOREM II. // F, G are defined as before, and if each depends 
on a parameter, % , the relation 

(8) J'ft; a?,,..-, x^ + Oft; y u , 2/n) = J x r y r 

T=l 

being an identity, because of T or T~ l , either in the n + 1 arguments 
( ; #!,, Xn) or in the n + 1 arguments ( ; y ly , y n 



Let ( ; !,, X B ) be the independent variables in (8). Then 



= 

y r ft & ft' 
But 



and the proof is complete. 



342 MECHANICS 

3. Proof of Hamilton's Equations. We start out with the 
Lagrangean Function L(q r , K T , t), which fulfils the condition : 

'"' L 



w n(if if } 9 

V \ K li ) K m/ 

and make the transformation : 

(2) p r = -, r = 1, , m. 

The Hamiltonian Function // (q r , p r , f) is then defined by the 
equation : 

(3) L + H = % p r K r . 

T 

If, then, we set x r K r , y r = p r , and regard the q r and t as 
parameters, all the conditions of the theorems of 2 will be met. 
It follows, then, that the inverse of (2) is given by the equation : 

and furthermore that 

(5; + g^ ~ t r ,--, m. 

It is also true that 

dt dt ' 

although this relation is not important for our present purposes. 
Turn now to Lagrange's Equations : 

dq, 
~dt 

d <9L _ cuu 

dt d* r dq r 

The first of these, combined with (4), gives : 

m dqr - m r-\ m 

\OJ , ~ , / 1,, III. 

From the second, combined with (2) and (5), we infer that 

(9) -37- = -r- , T = 1, , m. 



HAMILTON'S CANONICAL EQUATIONS 343 
But these are precisely the Hamiltonian Equations (5) of 1 : 

dqr_9H dpr__3H 

dt ~ dp r > dt - dq r > T ~ A ' ' ' 

which we set out to establish. 

The mathematical converse is simple. Given Equations (10) 
with the condition 



Equations (4) define a transformation, and then L is defined 
by (3). Then (2) arid (5) follow from the theorems of 2. And 
now the first of Equations (10), combined with (4), gives 

dq r . 

- = r = l,...,m. 

The second equation (10), combined with (2) and (5), leads to 
the equation : 

d dL _ dL _ 1 

~7i ~n ~^ t f 1> " " " ) W" 

dt 8K r dq r 

Thus wo arrive at Lagrange's Equations (7). 

We see, then, that a knowledge of the function H is sufficient 
for a complete mathematical formulation of the motion. But 
what can we say of the physical meaning of // in the general 
case? There is an important restricted class of cases in which 
the definition is simple. Suppose there is a force function U 
depending on q r , t alone, and furthermore that the kinetic en- 
ergy T is a positive definite homogeneous quadratic form in the 
(/!,--, q m > Let L be defined by the equation : 

(11) L = T + U. 

Let K r = q r > Then 



The transformation : 

8L 

*-aT r 

now becomes : 



344 MECHANICS 

Thus 

?,,- 2 ,j-2T. 

r = l r c/ " r 

Hence 

(12) ff = J) p r * r -L = T-U. 

T 

Still more specially, if neither T nor [7 depends on t, then // 
becomes the total energy of the system. That H is here constant 
along any given path appears as follows. We have in the general 
case the relation : 

dH m 



as is seen at once by differentiating : 

*H = VM^: + T?dH_dpr , BH 

dt $, d(Ir dt ^ dp r dt "*" dt ' 

and then making use of Hamilton's Equations. But in the gen- 
eral case dPI/dt ^ 0, and so H is not constant along an arbitrary 
path. If, however, H does not contain t, then 3H/dt = and 
since now dH/dt = 0, we have : 

(14) H = h. 



CHAPTER XII 
D'ALEMBERT'S PRINCIPLE 

1. The Problem. The general problem of Rational Mechanics, 
so far as it relates to a system of particles, can be formulated : 

i) in terms of the 3n equations given by Newton's Second Law 
of Motion : 
A) miXi = Xi, rmi/i = Y iy wz = Z it i = 1, - ,n ; 

ii) in terms of further conditions equivalent to 3n relations 
between the 6n + 1 variables (x i} y i} z iy X if Yi, Zi, t). A postu- 
lational treatment of these conditions will be found below in 
Appendix D. 

Two extreme cases may be mentioned at the outset. First, 
each variable Xi, Y iy Z if may be given as an explicit function 
of the Xi, yi, Zi and their first derivatives with respect to the 
time, and t : 

X, = */ fa, y t , z if Xi, y iy z { , t) 

YJ = */ fa, y iy Zi, i, y i} Zi, t) 



Thus A) reduces to a system of simultaneous differential equa- 
tions for determining Xi, y iy Zi as functions of the time, and with 
the solution of this problem the determination of the Xi, Yi, Zi 
is given by substitution. 

Secondly, at the other extreme, the path of each particle and 
the velocity of the particle in its path may be given. Thus 
#ij y\> Zi become known functions of t, and again the Xi, F t , Zi 
are found by substitution. 

Between these two extremes there is a class of problems in 
which constraints occur which can be eliminated by a general 
principle due to d'Alembert. We shall not attempt to give 
a general definition of " constraints/' for no such definition exists ; 
but we can formulate a requirement which embraces the ordinary 
cases that arise in practice. Let 8x it dyi, 6z t be any 3n quantities 

345 



346 MECHANICS 

whatsoever. Then it is seen at once from A) that the following 
equation is true : 

(1) 2) ( m & ~ x *> * x * + ( m *y* ~ r ) fy< + ( m <*< - z *> dZi = - 
-i 

This equation is sometimes referred to as the General Equation 
of Dynamics. 

Now it may happen that the force X^ F, Zi can be broken 
up into two forces : 

(2) Xi = XI + X!, Yi = Y( + Yl Zi = Z( + ZI 

where the two new forces, namely, the X' it F, Z\ and the 
X* t F|*, Z*, are simpler than the old for the following reasons. 
i) The X't, Yi, Z{ are either explicit functions of the x^ ?/, Zi, 
i, yi f Zi, t or they involve in addition a restricted set of un- 
known functions arising from forces which are not given as func- 
tions of these &n + 1 variables. 
ii) The Xf, Yf, Zf have the property that 

(3) 2) XfdXi + Yfdyi + ZfdZi = 

!--=! 

for all values of the 6xi, 5t/, dz t which satisfy the \i equations : 

n 

(4) ^ / A ia dx i + B ia dyi + CieSz^ 0, a = 1, , M , 

<=1 

where the coefficients are given functions of the 6n + 1 variables 
Xi y yij Zi, Xi f j)i t Zi, t, and the rank of the matrix : 

"11 " * " -"nl 

(5) ' 



is /x ; and conversely. 

By means of- Equations (4) the 3n quantities X*, Yf, Z* can 
be expressed in terms of /x unknowns as follows. Multiply the 
a-th Equation (4) by an arbitrary number \ a , and subtract the 
new equation from (3). Thus 



(6) 2) (ft - 



i-l a-l 



D'ALEMBERTS PRINCIPLE 347 

Now, in Equations (4), a certain set of 3n n of the &c, By*, dZi 
can be chosen at pleasure and then the remaining /* of these 
quantities will be uniquely determined, for at least one At-rowed 
determinant from the matrix (5) does not vanish. It follows, 
then, that \, , X^ can be determined uniquely from a suitable 
set of ju equations chosen from the 3n equations : 

H M f- 

(7) X* 2^ Ai a \ a , Yi 

a= 1 

And now the remaining 3n /z Equations (7) will be satisfied 
by these values of the X's. For Equation (6) has become an 
equation in which only those terms appear for which 6x,, 8yi, 6z 
are arbitrary, and hence their coefficients must each vanish. 
Equations A) can now be written in the form : 

(8) mix* = X( + 5) A ia \ a , nnyi = Y( + J fi ia X, 



where the X t , , X^ have come to us as linear combinations 
of /z suitably chosen X*, Y* 9 Z*. On the other hand, they appear 
in Equations (8) merely as /z unknown functions, which can be 
determined from /* of these equations and then eliminated from 
the remainder. 

Virtual Work. To put first things first was never more impor- 
tant than in the statement of d'Alembert's Principle. The 3n 
quantities 8xi, Sy iy dZi are to begin with 3n arbitrary numbers, 
and we then proceed to restrict them by the equations (4). Never- 
theless, whatever values they may have, they determine by defi- 
nition a virtual displacement of the system of points (Xi, t/, 2,-), 
and the quantity : 

W s - 2) X { dxi + Yi By* + Z, dZi 

=i 

is by definition the virtual work corresponding to this virtual 
displacement. Thus Equation (3) says that the force X* t Y*, Z* 
is such that it does no virtual work when the virtual displacement 
is subject to the conditions (4). 



348 MECHANICS 

D'ALEMBERT'S PRINCIPLE FOR A SYSTEM OF PARTICLES. Given 
a system of particles, the motion of which is determined in part by 
Equations A). The discovery of an analysis of Xi y Yi, # by (2) 
and of the most general virtual displacement 5Xi, dy^ 6z if whereby the 
virtual work of the force Xf, Yf, Z* vanishes, this virtual displace- 
ment being expressed by (4); finally the elimination of dXi, dy if dz ir 
and X*j Yf, Z*, as above set forth, whereby 3n n equations free 
from these unknowns result; this is the spirit and content of 
d 'A lembcrt's Principle . 

This enunciation of the Principle does not represent its historic 
origin, but rather its interpretation in the science today ; cf . 
Appendix 1). 

2. Lagrange's Equations for a System of Particles, Deduced 
from d'Alembert's Principle. Let the coordinates x, yi, z of the 
system of particles considered in 1 be expressible in terms of m 
parameters and the time : 



(D 



i?m, 

, <im, 

i tfm, 



where (q l} , q m ) is an arbitrary point of a certain region of 
the (</!, , g m )-spacc and the rank of the matrix is m. Let 



Then by the purely mathematical process of differentiation and 
substitution Equation (1) of 1 yields : 



dT 8T 

ZdtWr'Wr 

where 



and 
(4) 



Now, the m quantities 6q l9 , dq m are wholly arbitrary. Hence 
the coefficient of each term in (3) must vanish, and so we arrive 



D'ALEMBERT'S PRINCIPLE 349 

at Lagrange's Equations in their most general form for a system 

of particles : 

,,, d 8T 8T 



Here, no restriction whatever is placed on the forces X, F t , 
nor is the number of q r '$ required to be a minimum. 
In an important class of cases which arise in practice, 

(6) x, = x'< + xi F, = F; + 17, Zi = z; + z*, 

where 



Hence 



r = 1, , TW. 

Equations (5) now become Lagrange's Equations for this restricted 
case. The cases of constraints that do no virtual work are here 
included. Cf. further Appendix D. 

3. The Six Equations for a System of Particles, Deduced from 
d'Alembert's Principle. Let the system of particles of I be 
subject to internal forces such that the action and reaction between 
any two particles are equal and opposite and in the line through 
the particles : 



X* 
ij __ 

~ 



And let any other forces X' tj Y[, Z( act. Let 

dXi = a + pz t - yiji 
fyi = b + yxi aZi 
dZi = C + ayi - pXi 

where a, 6, c, a, /?, 7 are six arbitrary quantities. Since the 
internal forces destroy one another in pairs, and likewise, their 
moments, Equation (1) goes over into the following: 



350 MECHANICS 

= a J (m,< - X' ( ) + b 2 (*<#< - F|) + c 2 (<*< - Zf) 



18 2) ( 
x 



Now, set any five of the six quantities a, 6, c, a, #, 7 equal to 0, 
and the sixth equal to 1. Thus the six equations of motion, 
from which the internal reactions have been eliminated, emerge : 



(1) 



n n 

) m * g = 2J 



In vector form these equations appear as the Equation of Linear 
Momentum : 

^ = F 
and as the Equation of Moment of Momentum : 



dt 

We have used d' Alembert's Principle to deduce a set of necessary 
conditions. These are not in general sufficient, because the fore- 
going choice of dx if 8y iy dzi is not in general the most general one. 

4. Lagrange's Equations in the General Case, and d'Alembert's 
Principle. Consider an arbitrary system of masses, to which 
Lagrange's Equations, on the basis of suitable postulates, apply : 

/i\ d dT dT n i 

(1) 5 a --" r-i,..-,*. 

If we set by way of abbreviation : 

(2) ddT _dT _ 

(2) ~ [ ^ 



D'ALEMBERT'S PRINCIPLE 351 

then 

(3) 2 ([71 - Qr) Sq r = 0, 

where dq l9 , dq m are any m quantities whatever. It may 
happen that Q r can be expressed in the form : 

Qr = Q'r + Q], 

where Q' r is for some reason simpler than Q r and where, moreover, 

(4) Qffy, + + Q;s? m = 0, 
provided 

(5) daidqi + ' ' + a>am8q m = 0, a = 1, , /I, 

the rank of the matrix : 



being /*. By reasoning precisely similar to that used in 1, it is 
seen that the Q* can be represented in the form : 

M 

Qr 2L a <*r^a, r = 1, , W, 



where the X can be interpreted physically as certain linear com- 
binations of a suitable set of /* of the quantities Q* . 
Moreover, Lagrange's Equations take on the form : 

d dT dT , A _ 



where now the X a are thought of as unknown functions, which 
can be determined by /* of these equations and then eliminated 
from the remaining m n equations. 

Virtual Work. In all cases the expression 



can be interpreted as the virtual work done on the system by the 
forces which correspond to the Q r . In particular, then, the 
condition (4) means that the virtual work of the forces which 
lead to the Q* is nil, provided that the virtual displacement cor- 
responds to the condition expressed by Equations (5). 



352 MECHANICS 

5. Application: Euler's Dynamical Equations. Consider a 
rigid body, one point, 0, of which is fixed, and which is acted on 
by any forces. Its position may be described geometrically in 
terms of Euler's Angles, Chapter VI, 15 : 

(1) Qi = 0, q 2 = t, q* = <p. 
Its kinetic energy is, by Chapter VII, 6 : 

(2) T = -i (Ap* + Bq* + Cr 2 ), 
where 

p = \j/ sin 6 cos <p + 6 sin <p 

(3) q = \l/ sin 6 sin (p + 6 cos <p 
r = ^ cos + ^ 

By d'Alembert's Principle, 4 : 



where all three 5^ r are arbitrary. Let 5q { 0, dq 2 = 0, 
Compute 



The value is seen at once to be : 



On the other hand, Q 3 can be computed as follows. Denote 
the vector moment of the applied forces, referred to 0, as 

M = La + Mf3 + Ny. 

Then the virtual work corresponding to the virtual displacement 
(5q ly 8q 2) 5g 3 ) = (0, 0, dq z ) is seen to be : 



Hence Q 3 = N, and we find : 



Thus one of Euler's Dynamical Equations is obtained, and 
the other two follow by symmetry, through advancing the letters 
cyclically. 



D'ALEMBERT'S PRINCIPLE 353 

The reader will say : " But this is precisely the same solution 
as that given earlier by Lagrange's Equations, Chap. X, 16." 
True, so far as the analytic details of the solution go ; and this is 
usually the case with applications of d'Alembert's Principle. It 
is the approach to the problem through the General Equation 
of Dynamics, 1, which here yields (4), and the concept and use 
of virtual work, that brings the treatment under d'Alembert's 
Principle. 

6. Examples. Consider the problem of the ladder sliding 
down a smooth wall; cf. Fig. 88, p. 147. Let us regard this 
problem as the motion of a lamina, moving in its own plane. 
AH the generalized coordinates of the lamina we may take the 
coordinates of the centre of gravity : 

?i = x, q 2 = y, q z = 8. 
Then 

(1) T = %M(fr + p) + pf F 2 , 

where k is the radius of gyration about the centre of gravity. 
By d'Alembert's Principle, 

(2) 2 ([T\ r - Q r ) 8q r = 0. 

r-l V ' 

In the present case, 

Q^ = S5x, Q 2 6</ 2 = (R - Mg) by, 

Q 3 5<7 3 = a (S sin - R cos 6) d6, 
and thus Q r is determined. Let 

Qr = Q; + QM 

where 

Q* = s, Ql = R, Q 3 * = a OS sin 9 - R cos 8). 

Now, x, y, 6 are connected by the relations: 

(3) x = a cos 0, y = a sin 6. 

If, then, we subject dx, dy, SO to the corresponding relations: 

8x = a sin 6 60, 6?y = a cos 60, 
we see that 

(4) Qr^i + Ql 5<7 2 + Q,*ff, = 0. 



354 MECHANICS 

Thus the virtual work of the forces Q?, corresponding to such 
a displacement, is seen to be nil, and so Equation (2) is replaced 
by the simpler equation : 

(5) i; (m, - $W == o. 

r-l V ' 

Hence 



M^j(- a sin 0) 66 + (^^f + Mg) a cos 6 69 + MW 66 = 0. 

On replacing these second derivatives of x and y by their values 
from (3) a differential equation in the single dependent variable 
is obtained : 



and this determines the motion. 

Rough Wall. Suppose, however, the wall is rough; Fig. 145, 
p. 323. Equations (1) and (2) still hold. But now 

Qi*fc = (S ~ R) x, Q 2 6q 2 = (R + S - Mg) 8ff, 
Cs ^3 = a [S (sin 6 + /z cos 6) + R (/x sin 6 - cos 0)] 66. 
Let 

Q r = Q; + Q;, 

where 

Qr = S - /, Q* = B + MS, 

Q* = aS(sin + M cos 0) + aR(n sin cos 0). 

The values of 5^ D 6q 2 , 8q z which make the virtual work of the 
force Q* vanish : 

QI^ + c;?i + cr?i = o, 

are found by making the coefficients of B and S zero in this last 
equation : 

/z&7i + 6q 2 + a (M sin 6 cos 0) 6q z = 



. .. 4- a (sin + M cos 0) 6q 3 = 
Hence 

f (1 + M 2 ) fyi = a [ (1 - /i 2 ) sin - 2M cos 0] 6q^ 
I (1 + M 2 ) 5^ 2 = a [- 2M sin + (1 - M 2 ) cos 0] 6q 3 



D'ALEMBERT'S PRINCIPLE 355 

Equation (5) now becomes : 



M^jSq, + (M^JL + Mg) Sq, + Mk^dq, = 0, 

and it remains only to substitute the values of 5q lf 8q 2 from (7), 
and the values of x, y from (3), and reduce. The result is : 



((1 - M 2 ) a* + (1 + M 2 ) *) JJ + 

ag [2/x sin 6 - (1 - /* 2 ) cos 0]. 



The virtual displacement (dq lt 5g 2 , dq^) which here led to the 
elimination of the unknown reactions R, S was not one which 
in any wise conformed to the " constraints " in the sense of the 
floor and the wall. If we replace R and /z# by their resultant 
and draw a line L through the bottom of the ladder perpendicular 
to it, and then do the same thing at the top of the ladder, thus 
obtaining a line L 2 , the above virtual displacement corresponds 
to an actual displacement in which the bottom of the ladder is 
moved along L t and the top along L 2 . 



CHAPTER XIII 

HAMILTON'S PRINCIPLE AND THE PRINCIPLE 
OF LEAST ACTION 

1. Definition of 8. A new and independent foundation for 
Mechanics is given by Hamilton's Principle and certain other 
Principles of like nature. An integral, for which Hamilton's 

Integral : 

j 

V + t/) dt, 

is typical, is extended along the natural path of the system, and 
then its value is considered for a neighboring, or varied, path. 
The Principle asserts that the integral is a minimum for the 
natural path, or at least that the integral is stationary for this 
path, i.e. that its variation vanishes : 



(T + U) dt = 0. 



It is to the treatment of this subject that we now turn. Obvi- 
ously we must begin by defining what is meant by a varied path 
and by a variation 8. 

Let F(x l9 , x n > x[, - , x' n , u) be a function of the 2n + I 
variables indicated. Here, (x l9 , x n ) shall lie in a certain 
region R of the n-dimensional space of the variables (x ly , x n ) ; 
the variables x[ 9 , x' n shall be wholly unrestricted ; and u 
shall lie in the interval : a g u g b. The function F shall 
be continuous, together with its partial derivatives of the first 
and second orders.* Let 

*As regards assumptions of continuity, we lay down on GO and for all the 
requirement that whatever arbitrary functions are introduced shall be continuous, 
together with whatever derivatives we may wish to use, unless the contrary is 
stated. 

For an introductory treatment of the Calculus of Variations cf. the author's 
Advanced Calculus, Chap. XVII. 

356 



HAMILTON'S PRINCIPLE. LEAST ACTION 357 

C : Xi = Xi(u), a ^ u g 6, i = 1, , n, 

be a path lying in R. Let 

, _ dxj(u) 
Xl ~ du ' 

Thus a path T in the (2n + l)-dimensional space of the arguments 
of F is determined. 

By a varied path, F', is meant the following. Let C f be a curve 
in R defined by the equations : 

C' : Xi = Xi(u, e), a ^ u g 6, f = 1, , n, 

where 

a?t(w, 0) = Xi(u), 

and is considered only in a region for which | e | is small. De- 
note partial differentiation with respect to u by d. Let 

, e) // \ -i 





' ~~ du ' ' , , , 

be chosen as the values of the #(,-, #. The curve F' in the 
(2n + l)-dimcnsional space is what is meant by a varied curve. 
The variation of #,-, or &c,-, is defined by the equation : 



Since x l (u, e) is any function that conforms merely to the general 
requirements of continuity, we see that 

dxi = IH(U), i = 1, , n, 

is a wholly arbitrary function, restricted only by the above re- 
quirements of continuity. 

The variation of x' t , or bx( is not, however, arbitrary, but is 
defined by the equation : 



dude >o 
Thus 



Hence 



. A < 
-r--oa; = o-j 
du du 



It is now natural to lay down the further definition : 
(4) 



358 MECHANICS 

Definition of SF. By the variation of F (a;,-, x' t , w) is meant : 

8 "=().., 

where Xi and xj on the right-hand side are set equal to x (u, 
and ZI'(M, e). Hence 

(6) ^-|(J>' + I 

It is obvious that 

8(F + $) = 8F + d$; 



and also that 



where 

, ,*,,, x'n, u), k = 1, , m. 



Finally, the definition : 

(7) ddF = ddF, 
corresponding to the theorem : 

/ON * dF d8F 

(8) a 5?-"5T 

And similarly, 

6 b 

(9) J FSd* = * 

a a a 

The dependent variables x^u), , x n (u) play a r61e in the 
foregoing definitions analogous to that of the independent variables 
in partial differentiation. But the analogy holds only up to a 
certain point, and to assume it beyond theorems like the above 
formulas which we can prove, has led to confusion and error in 
physics. 

Variation of an Integral. Consider the integral : 

b 

/ f 
F(Xi, u ' ' > X H9 X 19 , X n , U) du, 



HAMILTON'S PRINCIPLE. LEAST ACTION 359 

taken along the path F. By 8J is meant the following : Extend 
the integral along the path F'. Thus a function /(e) is defined. 
and now, by definition : 



(10) ^ 

It follows at once as a theorem that 



(ID 

The integral is said to be stationary for a particular path F if 

b 

8 CFdu = 0, 

a 

no matter what functions 8x* = t m(u) may be. The condition 
is readily obtained in case dxi is restricted to vanish for u = a 
and f or u = 6 : 

(12) dxi | . = in (a) = 0; &e< | Ussb = ^(6) = 0. 

For: 

d ( $ F ^ \ dF f i d ^ * 
d^ V^J 5X V " ~d$ 8Xi + dH W< 8Xi ' 
Hence 

03) 

If, now, the integral in question is to vanish for an arbitrary 
choice of &C;, it is easily seen that each parenthesis in the inte- 
grand of the last integral must vanish, or : 



These are known as Euler's Equations. 
It is clear that 

6 b 

(15) d jFdu= j8Fdu. 



360 MECHANICS 

The limits of integration may be varied, too. Let 



a' = ^(a, ), 6' = *(&,), 
where ^?(a, 0) = a, \f/(b, 0) = 6. Let 

6' 

J (c) = IF [Xi (u, e), x'i (u, c), u\ du. 

a' 

Then the variation of the integral is defined as before, by (10). 
It follows that 

6 b 

(16) dCFdu = C6Fdu + F(B i9 B f i9 b 

a a 

where 
. A* = z(o), A'< = x(a), < 

EXERCISE 

Since 

l/, 6) 



it follows (under the ordinary hypotheses of continuity), on let- 
ting e approach 0, that the right-hand side approaches 

f. 

du 
The left-hand side approaches 8&. Hence 

,eM> d 
5 -j- = -7- 6$. 
aw aw 

Thus Equation (7) is obtained as a theorem, and no new definition 
is necessary. Explain the error. 

2. The Integral of Rational Mechanics. All that has gone 
before merely leads up to the definition of the variation of the 
following integral : 

ti 
(1) j > F(x lt ---,x n ,x l ,-",x n ,()dt, 



HAMILTON'S PRINCIPLE. LEAST ACTION 361 

where the limits of integration may be constant or variable. The 
answer would seem to be simple, since t is the variable of integra- 
tion and hence the independent variable in each of the functions 

Xi = Xi(t). 

But the symbol written down as the integral (1) is taken in Physics 
to mean something totally different. Let 



(2) t = t(u), ^ u 

be any function of u such that, in the closed interval (0, 1), 

0<f -f. 

du 

Then the symbol (1) is taken to mean the integral : 

(3) / = JF (x lt ,*, |f, ..-, |?) t'du, 



where x[ = dxi/du, and the "variation of the integral (1)" is 
understood to be the variation of this last integral. Thus 

(4) dJ = Cd(Ft')du, 

o 

where u is the variable of integration, and the independent vari- 
able in each of the functions Xi = Xi(u), t = t (u). 

This last variation, (4) : &/, comes under the earlier definition 
of the variation of an integral. In particular, Equation (4) may 
be written in the form : 

8J = 



In each of these integrals the variable of integration may be 
changed back from u to t, and thus 

t <t 

(5) SJ = CdFdt+ foddt. 



fbFt'du+ CF8t f du. 



362 MECHANICS 

The variation of t, namely St, is an arbitrary function of u : 

U = T(M), 
and 

dSt T'(U) 
dt t'(u)' 

where u is the inverse function defined by (2). Moreover, by 
6F in (5) is meant the following : 



m - 

where 

/z,'\ t'5x' t - xW , d .., d 

8 (7) = - ?5 . *, = Tu $x<, st = ^ a. 

We see, then, that 

' 



Now, when 2 is the independent variable, 

/o\ *- d dXi 

(8) 5^* = - ir - 

The two formulas, (7) and (8), show that 5i is not invariant 
of the independent variable. Why should it be? Similarly, 
the variation of an integral is not invariant of the variable of 
integration. Much of the confusion in the literature arises from 
losing sight of this fact. The " variation of the independent 
variable" is supposed to cover this case. It does so when and 
only when it becomes identical in substance with the above 
analysis. 

3. Application to the Integral of Kinetic Energy. By defini- 
tion, the kinetic energy 



Hence 

n 

(1) &T = 5} mi(idXi + yifoji 

i-i 

no matter what the independent variable and the dependent 
functions may be. If the former is u } then 



HAMILTON'S PRINCIPLE. LEAST ACTION 363 



(2) 8T = ,[*, 5 () + fr S () + 6 

By Formula (7) of 2 and the corresponding formulas involving 
y iy Ziy this equation becomes : 

a, w. 



Variation of the Integral : 
(4) J = 



Let the natural path in space be represented parametrically by 
the equations : 

Xi = Xi(u), ^ u ^ 1, 

and let 



The variation of this integral has, by 2, (5) the value : 

(5) 

By the aid of (3), 



f*Tdt= (*8Tdt+ CTdd 

*o to t 



The first term on the right can be transformed by integration 
by parts, the integrand obviously having the value : 



Hence 

*t <i 

(7) fdTdt=-Cj? rm (Xi dXi + Hi dyi + 2< 62^) d< 

V V < " 1 

'l 

+ 5) wiifofa, + yi% + ^fe { ) tl ~ 2 TlTd^. 

< . i <o J 



364 MECHANICS 

Finally, then : 

/i ^ 

(8) 5 CT dt = - / 5) m t (ft fa, + 

i:sl 



The variations dxi, dy^ bz^ dt are 3n + 1 arbitrary functions, 
subject merely to the ordinary conditions of continuity. If, 
in particular, we impose on &c-, dy iy 5z t - the condition that they 
vanish at the extremities of the interval of integration, i.e. for 
t = t Q j t ly then 

*, / t <i 

(9) Ardt = - f 5) mi(ft fa* + *< + 2*820 * ~ 2 J 

/o 'o ~ *o 

and 

'' /! n 

(10) d (*Tdt =- f T m< (ft fa,- + y< fyi + 5f - 

/ / i-i 

/O h 

4. Virtual Work. By the virtual work of the forces Xi, F,-, Z t -, 
considered along the natural path : 

(1) Xi = Xi(u), yi = y(w), 2. = ti(u), UQ-^U ^ u ly 
is meant the quantity : 



(2) W s = 






where fai, 5i/i, 5^^ are 3n arbitrary functions of u, subject merely 
to the ordinary conditions of continuity. 

This quantity is often denoted by dW ; but it is not, in general, 
the variation of any function, and so it is better to avoid this 
confusion, writing 5W only when W 8 is the variation of a function. 

6. The Fundamental Equation. Combining Equation (9) of 
3 with Equation (2) of 4 we have : 



HAMILTON'S PRINCIPLE. LEAST ACTION 365 
(1) 



Here the 3n + 1 variations &r t -, 6?y t , 5z t -, 5 are arbitrary except 
that the first 3n of these vanish for t t Q , ^ ; and the n forces 
Xi, Y{, Zi are any forces whatever. If these are the total forces 
acting on the particles, the right-hand side of (1) will vanish since 
each parenthesis vanishes by Newton's Law, and we shall have : 

t\ 
(2) J(ST + 2T < ~ + W t ) dt = 0. 

h 

Let the total force be broken up into two forces : 

(3) Xi = xi + xi Y> = y; + Y;, z, = z; + zi 

Then 

(4) W s = W v + W s *. 

Suppose that W&* vanishes : 



(5) W 8 * = X;txt + Yt8y { + Ztdz< = 0, 

t=i 

when the variations dX{, 8yi, dzi are chosen subject to certain 
conditions. Then Equation (2) takes the form : 



(6) 



where now dxt, 8yi, dzi satisfy these conditions, dt being still wholly 
arbitrary, and 

(7) W 9 = 2) XJ 



t=i 
These conditions usually take the form : 



(8) 



366 



MECHANICS 



where A ta , B ta , C ia are functions of x,-, /<, Zi, x it y f , z it t, and the 

rank of the matrix : 

A n C n i 

(9) 

* 1 I/A * * * v> n/A 

is M. This case includes both the holonomic and the non-holo- 
nomic cases. But it must be observed that 8T is in general no 
longer, or not yet, the variation of a function.* 

Generalized Coordinates. Suppose that the coordinates x t -, y i} Zi 
of each mass mi can be expressed in terms of m parameters 
q.u ' ' ' i q an< i th e time : 

Xi = fi(q\j > qm, f) 

Vi ~ <?i(qu ' i q*n, 

Zi = ^i(q^ , q mj t) 
where the rank of the matrix 



(10) 



is m. Suppose further that Equation (5) is satisfied when 

dfi s , , dfi , 

OXi == 7 OQ'i ~i~ " * * H O^m 

^^j ^Q'm 

*. _ ^ ^ . . fa * 



(11) 



the 5^, , 8q m being arbitrary. Let 

/1O\ /^ ''O ( V ^i I V/ ^2/ I ^ 

(12) Q r = > ( A< -r + Yi -r + / 



+ I*-'**. 



r = 1, , m. 



* The definition of the variation of a function, it will be recalled, is based on 
the dependence of the latter on certain arbitrary functions, whose variations may 
also be taken as arbitrary. These arbitrary functions are analogous, let us repeat, 
to the independent variables in the case of partial differentiation. And so further 
assumptions (i.e. postulates or definitions) are needed before dT can again mean a 
variation. 



HAMILTON'S PRINCIPLE. LEAST ACTION 367 

Then 

(13) W? = Q! & + +Q m Sq m . 

On the other hand, 

(14) T = T(q l9 ,.,*, ,&,,<) 



and 5T 7 as given by 3, (2), becomes the variation of this latter 
function, where qi(u), , q m (u), t(u) are the independent 
functions. Equation (6) of the present paragraph now takes the 
form: 



where dT means what it says the variation of T and where 
W s is the W y of (13). 

We will denote this equation as the Fundamental Equation. 
It embraces Equation (2) above, for the Xi, t/, z can always be 
taken as m = 3n generalized coordinates. 

This equation is sometimes written in the form : 

ti 
X) C(dT + 5W) dt + 2T 8dt = 0, 

where 

(15) dW = Q l dq l + -- +Q m dq m . 

Let us see just what this means. First of all, the equation is 
true under the hypotheses which led to Equation I. These were, 
that the path is the natural path of the system, given by the 
equations : 

(16) q r = ffr(tO, t = t(u), 
where (0) = t , t(l) = t lt and the variations 

8q r = ir(u), 8t = / (w), 

are arbitrary functions subject merely to the conditions : 
7? r (0)=0, r = 0, 1, ...,m; r? r (l) = 0, r = 1, , m, 



368 MECHANICS 

and possibly to a further restriction : 

I rj r (u) | < A, | j r (u) | < h, r = 0, 1, , m, 

where h is a definite positive constant. 

Furthermore, in Equation X), 8W = W$ is not in general the 
variation of any function of q lt , q m , t. The Q r have definite 
values at each point of the natural path, and so are definite func- 
tions of u; but they do not in general have any meaning at a 
point (q r , t) not on the natural path, nor does dW. 

Finally, 

(17) ^SfV 

where 



^ 
\du du du du \du 

The last term in the integral has the value : 



/27 





And now the meaning of Equation X) is this : If q r and t 
are set equal to the functions (16) which define the natural path 
and if dq r , 8t are chosen arbitrarily, subject merely to the general 
conditions above imposed, Equation X) will be fulfilled. Thus 
Equation X) expresses a necessary condition for the motion of 
the system and this in all cases, be they holonomic or non- 
holonomic. 

Since Equation X) is true for all variations 8q r , 8t, it still repre- 
sents a necessary condition when these functions are subject to 
any special restrictions we may choose to impose on them. For 
example, it may happen that the Q r can be broken up into two 
functions : 

Qr = Qr + Qr*, r = 1, , m, 

such that 

QiiQi + + Qlfym = 0, 
provided that 

a*i8qi + + Oamfyw = 0, a = 1, , /i, 



HAMILTON'S PRINCIPLE. LEAST ACTION 369 
where a ar = a ar (q l9 , q m , q lf , q m , 0> an d the rank of the matrix : 



is IJL. Here, dW is replaced by 



(18) 



5W = 



+ 



but only m /i of the &/ r , and dt, can now be chosen arbitrarily. 
In what sense is 5T now a "variation"? Emphatically, in no 
sense ; for no definition has been laid down which reaches out 
to this case, and it is only from a definition that 5T can derive 
its meaning. Nevertheless, Equations (17) and (18) continue 
to define the values of the terms dT, bW that appear in Equa- 
tion X), and thus this equation continues to have a meaning, and 
to hold when a certain set of m /* variations 8q r , and dt, are 
chosen arbitrarily. 
Force Function. Finally, there may be a force function, U : 



(19) 



where U is a function of the #,-, y^ z, and t. Thus the Funda- 
mental Equation (2) becomes in this case : 



II. 



where the (Xi, F<, Zi) of (19) is the total force acting on m,-, 
provided (/ does not depend on t ; otherwise we must understand 
by d(J the virtual variation of U, or : 



Again, there may be a function U(q l , , q m> <) such that 
in (15) 

SU 



r 1, 



m. 



Then 



&W = BU 



370 MECHANICS 

and the Fundamental Equation takes on the same form, II., 
provided U does not depend on t ; otherwise, 

' U ~W * + ~'+W t *" 

oq\ oq m 

6. The Variational Principle. The variational principle as ex- 
pressed by the Fundamental Equation I. of 5, or even by 
Equation II., does not assert that the integral of some function, 
or physical quantity, is a minimum, or even stationary : 

5 I (something) =0 or Id (something) = 0. 

For the integrand is not a variation, in the sense of the Calculus 
of Variations; nor are the forces of the problem varied; they 
are considered only along the natural path of the system.* The 
Principle expresses a necessary condition for the motion of the 
system. In the non-holonomic case, the condition cannot be 
sufficient, since the first-order differential equations have not 
been incorporated into the formulation of the problem. 

We turn now to certain further restrictions whereby Hamil- 
ton's Integral or an analogous integral does become stationary, 
and in fact, in a restricted region, a minimum. 

7. Hamilton's Principle. If we set : 

t(u, c) = U, t Q ^U^ t lt 

then 

8t s 

and the Fundamental Equation I. becomes : 



(1) 



We can now suppress the parameter u since the time is not to be 
varied. 

* In its leading ideas this treatment was given by Holder, Gottinger Naehrickten, 
1896, p. 122. Unfortunately Holder felt impelled to defer to the primitive view of 
variations as " infinitely small quantities" in the sense of little zeros, i.e. infinitely 
small constants or functions of Xi, y lt z, t. In the foot-notes on pp. 130, 131 the 
"neglect of infinitesimals of higher order" renders obscure in fact, vitiates 
the treatment, so far as clean-cut definitions go. The writer cannot but feel that 
the inner Holder would have preferred such a treatment as that of the text, but 
that he did not have the courage to break with the unsound traditions of the little 
zeros, for fear of losing his clientele. 



HAMILTON'S PRINCIPLE. LEAST ACTION 371 

Suppose that a force function U exists, which depends only 
on the Xij 2/, z and t, or on the q r and t : 

(2) U=U (x if y<, z iy f) or U = U (q r , t). 

Since t is here the independent variable with respect to variation 
5, we have 

W 8 = 6U 

in the sense of the Calculus of Variations, and (1) becomes : 



*i 
(3) C(ST 



= 0. 



It must be remembered, however, that the variations &r,, fly,-, 
bZi or 5q r satisfy the condition of vanishing when t = t and when 
t = t 1 . 
Here we meet our first example of an integral, 



(4) 

to 

the variation of which vanishes : 

ti 
(5) * f(T + U) dt = 0. 

h 

This equation embodies Hamilton's Principle, which we may 
formulate as follows. 

HAMILTON'S PRINCIPLE. Let T be the kinetic energy of a system 
of particles f and let a force function U = U(q r , t) exist. The 
natural path of the system is that for which Hamilton's Integral: 



(6) l(T + U)dt, 
is stationary: 

(7) d I (T + U) dt = 0. 



Here t is the independent variable, and the variations of the dependent 
variables are such as vanish when t = t Q and when t = t v 



372 MECHANICS 

A necessary and sufficient condition that (7) be true is afforded 
by Euler's Equations, 1, which here become : 

d dT dT dU , 

_ __ ______ rp . 1 , , . i*jj 

dtdq r dq r ~ dq r ' ' ' 

But these are precisely Lagrange's Equations for the system. 
Incidentally we have a new proof of Lagrange's Equations, in 
case we make Hamilton's Principle our point of departure. 

We have proved the Principle for systems of particles with m 
degrees of freedom, and it can be established in certain more 
general cases, e.g. for systems of rigid bodies; provided each time 
that a force function exists. The case is also included, in which 
relations of the form : 

*>(?!> ' ' ' > ?, = 0, a = 1, , Ml 

exist ; cf . Bolza, Variationsrechnung, p. 554. The most general 
case is that of a system having a Lagrangean Function, or kinetic 
potential, L. In the above cases, 

L = T + U. 

When it is not possible to establish it without special postulates 
consider, for example, the motion of a perfect fluid or of an elastic 
body it is taken as itself the postulate governing the motion 
of the system. The Principle consists, then, in requiring that 

the Lagrangean Integral : 

d 

(8) fldt 

to 

be stationary ; or that 

i 

b Cldt = 0. 
V 

It will be shown in 14 that Hamilton's Integral (8) is actually 
a minimum for a path lying within a suitably restricted region ; 
but the minimum property does not necessarily hold for un- 
restricted paths. 

8. Lagrange's Principle of Least Action. Our point of departure 
is the Fundamental Equation II., 5, in which U now does not 
depend on t : 



HAMILTON'S PRINCIPLE. LEAST ACTION 373 

Moreover, T does not depend on t : 

T = T(qi, , q m , q iy ,?m). 
Thus we have : 

ti 

(1) C(ST + SU) dt + ZTddt = 0. 

<0 

Here each 5 represents a variation in the sense of the Calculus 
of Variations, the independent functions being q l9 - - , </ m , t ; 
but the integrand is not the variation of some function, nor is 
the integral the variation of some integral. Nevertheless, the 
equation is true when all m + 1 variations, q lt - , q m < t, are 
chosen arbitrarily. Let us examine more minutely the meaning 
of this last statement. These variations are defined by arbitrary 
functions : 

(2) 0r(u,e), (u,), 
such that 

q r (u,0) =g r (u), t(u,0) = t(u). 
Moreover : 

?r(0,) = <?r(0), ?r(l, =g r (l)j 



j(0, c ) = <(0, 0) = < = const. ; i(l, 0) = ^. 

But in general ^(1, c) ^ t v Thus 

5|-o = 0; ^| tt=1 ^ 0. 

In particular, then, the functions (2) may be restricted by any 
further conditions which are compatible merely with the general 
conditions of continuity. Such a condition is the one that, not 
merely for the natural path corresponding to = 0, but also for 
all varied paths : 

(3) T = U + ft, 

or, more explicitly : 

(3') T [ ?r (u, ), ^|] = U [ ?r (u, c)] + A, 

where fe is a constant. Since T is here a homogeneous quadratic 
polynomial in q lf - - - , q m , it is clear that t (u y e) is obtained by a 
quadrature when the q r (u,), r = 1, , m, are chosen arbi- 
trarily. 



374 MECHANICS 

Let 

be any function. By dF we shall now mean the following : 

(4) SF = - 

u 

where q r (u, e), t(u,e) are restricted by the relation (3), i.e. (3'). 
And similarly : 

(5) b \Fdu = -j- iFdu , 

J 0*J e-O 



where the integrand on the left is formed for the arguments 
q r (u), etc., and the integrand on the right, for q r (u, c), etc.; 
Equation (3') still holding. Thus it follows, in particular, that 

(6.) bT = 8U. 

Although these definitions are in form identical with the earlier 
ones, where the m + 1 functions (2) were arbitrary, they are in 
substance distinct, since these m + 1 functions are now related 

by (3')- 
Equation (1) now becomes, on suppressing the factor 2 : 

r, 

(7) CdTdt + Tddt = 0. 
Since obviously, under our new definition of 5, 

5 /T T /'\ xT 7 t f i rn jj^' 

0(1 1 ) = 01 'I -f- 7 Ot, 

and since 5t' = dbt/du, Equation (7) takes the form: 

i 

(8) I d(Tt')du = 0. 

o 
Hence, finally : 

(9) lj*Tdt = 0. 

We are thus led to the following Principle. 

LAGRANGE'S PRINCIPLE OF LEAST ACTION. Let a system of 
particles have the kinetic energy T and a force function U, where U 
depends only on the position of the system, not on its velocity or the 



HAMILTON'S PRINCIPLE. LEAST ACTION 375 

time, and where T is independent of t. Then a necessary and suffi- 
cient condition for the natural path of the system is, that 



(10) 



subject to the hypothesis that all varied paths fulfil the requirement 

that 

(11) T = U + h. 

In addition^ the variations of the coordinates shall vanish for t = t 
and t = Jj. 

The Principle thus formulated presents a Lagrangean problem 
in the Calculus of Variations with variable end points and one 
auxiliary condition : 



(12) 



CTM = o, 



The method of solution developed in that theory* employs 
Lagrange's Method of Multipliers. Briefly outlined it is as 
follows. Set 

F = T + \v, 

where X is a function of t, and let q r (t), X($), be determined by 
the m + 1 equations 

/*o\ *fl? d &F f\ t 

< 13 > Wr'dtWr^ ' '-I.'".*. 

and the second equation (12). From Equation (13) it follows 
that 

^ + X ^_^r^ + X 
tyr dq r dt Ldq r d 

or 



These equations, combined with the second equation (12), give : 
(14) X = - -J-. 

* Cf. Bolza, Variationarechnung, p. 586, where the case is considered that there 
are, in addition, relations between the coordinates, not involving the time. 



376 MECHANICS 

Hence the q r (t) are determined from the resulting equations, 

8T . dU d dT 



The latter are Lagrange's Equations. Incidentally we have 
a new deduction of them, based on Lagrange's Principle of Least 
Action. 

As in the case of Hamilton's Principle, so here we can give a 
direct proof of Lagrange's Principle of Least Action by means 
of the Calculus of Variations. For, as above pointed out, the 
Principle is equivalent to the Lagrangean problem represented 
by (12). 

Recurring to the condition (3) we see that the functions q l (u, e), 
' m ' 9 Qm(u, e) may be chosen arbitrarily, and the function t (w, e) 
then determined by (3'). If the function t(u, e) thus determined 
be substituted in the integral : 

i 

(16) fft'du, 



then t is completely eliminated from that integral. For 

(17) T=%A r .q r q., A T . = A. r , 

r. s 

the coefficients A r8l depending only on the q l9 - , q m . Now, 



/ = / 2r ' 

to 



(18) 

Let 
(19) 



where, as usual, q' r = dq r (u)/du. Then 



or 
(20) 

From (20) and (3) it follows that 
Tt' = 



HAMILTON'S PRINCIPLE. LEAST ACTION 377 
and thus t is eliminated, the integral (18) taking the form : 



f- 





We now have before us a problem in the Calculus of Variations, 
of much simpler type the simplest type of all, considered at 
the outset. It is the integral (21), formed for the functions 
q r (u), that is to be stationary, and these functions are all arbi- 
trary. After this problem has been solved, t is determined from 
(20), or 



(22) t-t, = f-j-JL 

J Vu 






This is Jacobi's Principle of Least Action, which we will treat 
in the next paragraph as an independent Principle. But it is 
interesting to see how it can be derived from the Fundamental 
Equation of 5, and proved as a particular case under Lagrange's 
Principle of Least Action. 

EXERCISE 

Show that Equation (1) under the restrictions named can be 
thrown into the form : 
<i 

dT , dU d dT\ ,, 

-x- h o 17 TT-) &Qr dt = 0. 

O(l r 0q r (It G(j[r' 

Hence deduce Lagrangc's Equations. 

9. Jacobi's Principle of Least Action. Let a system of particles 
have the kinetic energy T and a force function U, where U depends 
only on the position of the system, not on its velocity or the time, and 
where the conditions imposed on the coordinates do not contain the 
time explicitly. Then a necessary and sufficient condition for the 
natural path of the system is, that the integral : 

(1) fVU + hVTdt 

be stationary: 

(2) 




378 



MECHANICS 



The time is given by the equation: 
(3) T = U - 

or 



(4) 

where 

(5) 



r 



vir+T 



=Vrdt. 



where <h(u 
stationary : 



We can give a direct proof as follows. The integral (1) has 

the value : 

i 

(6) JVu + hVSdu, 



, q m (u) are arbitrary functions. It is to be 

i 

(7) d I VU + h VS du = 0. 



Hence Euler's Equations must hold, or : 

(8) (V(7 + h V5) 7 (V[J + h VS) = 0, 

T = 1, , m. 

d /vTT+1 



Hence 



. 



S d / 
du\ 



' 



Equations (9) determine the path ; t has not yet entered in 
the solution. Equations (3) and (5) now determine t; it is 
given by (4). 

It follows furthermore that 

dq r \du/ dq r y dq'r du dq r 

Combining these equations with (4) and (9) we find : 

/i i \ .__ . 

\ ' J4 O^, O^. Q 

at oq r oq r oqr 



HAMILTON'S PRINCIPLE. LEAST ACTION 379 

Thus we arrive at Lagrange's Equations. If we assume them, 
then we have a proof of Jacobi's Principle. Conversely, if we 
assume Jacobi's Principle, we have a new proof of Lagrange's 
Equations. 

10. Critique of the Methods. Retrospect and Prospect The 

symbol d is treacherous. It can and does mean many things, and 
writers on Mechanics are not careful to say what they mean 
by it. In d'Alembert's Principle the dxt, 8y if dZi began life by 
being 3n arbitrary numbers. In their youth they were dis- 
ciplined to conform to certain linear homogeneous equations. 
Thus still a number of them were arbitrary quantities; the rest 
had no choice, they were uniquely determined. 

Enter, the Calculus of Variations. And now the dxij dy^ dzi, 
and 8t become the variations of functions of a parameter, or inde- 
pendent variable, u. From now on these <$'s must be dealt with 
under the sanctions of the Calculus of Variations at least, 
if tho findings of that branch of mathematics are to be adopted. 

The Future. As the physicist fares forth over the uncharted 
ocean of his ever-expanding science, his compass is the Principles. 
He seeks an integral which in the new domain will do for him what 
Hamilton's Principle achieved in classical mechanics. There is 
mysticism about this integral. Imagination must guide him, 
and ho will try many guesses. But he will not be helped by an 
undefined d. He must make a cloan-cut postulate defining the 
integral, and then lay down a clean-cut definition of what he 
moans by tho variation. There is no short cut. A thorough- 
going knowledge of the rudiments of the Calculus of Variations 
is as essential in Mechanics as perspective is in art. 

11. Applications. Lot a particle be acted on by a central 
attracting force inversely proportional to the square of the dis- 
tance. Then 

(1) r = 

where the pole is at the centre of force, and it is assumed that the 
motion takes place in a plane (cf. Exercise 4, below). Then the 
integral : 



(2) f\ 



r*0'*du 



380 MECHANICS 

must be made a minimum. Set 



F (r, B, r', 0') = >(? + h )( r ' 2 + r2 *' 2 )' 
Then 

A ^ - ^ = n 
dw 00' 20 

Since dF/dO = 0, it follows that 

^ F - ^/M . . r*0' _ 

(6) W'-Vr + h Vr'* + r*0'* " 

If c = 0, then 

= const. 

and the motion takes place in a right line. But if c 7* 0, may 
be taken as the variable of integration : * u = 0, and (3) becomes : 



Hence 



e , . cdr 



*/; 



rVhr 2 + r - c 2 
Change the variable of integration : 

= 1 
"" r 
Then 

*=+/ 



/T i 22 

v Al ~| /it/* C 1L 

Performing the integration, we find : 

_ 1 e cos (0 y) = K 

EXERCISES 

1. Discuss in detail the case c = 0. 

2. In the general case, determine the constants e, K, y in terms 
of the initial conditions. 

* It is true that the interval for u was (0, 1) ; but it might equally well have 
been an arbitrary interval : a ^ u ^ b . 



HAMILTON'S PRINCIPLE. LEAST ACTION 381 

3. Obtain the time. 

4. Allowing the particle free motion in space, show that its 
path is a plane orbit. 

Suggestion : Use Cartesian coordinates. 

5. Discuss the motion of a particle in vacuo under the force of 
gravity. Assume the path to lie in a plane. 

6. In Question 5, prove that the path must lie in a plane. 

7. Explain the case of motion in a circle under the solution 
given in the text. 

12. Hamilton's Integral a Minimum in a Restricted Region.* 

THEOREM. The integral 



f 



(1) ldt 

to 

is a minimum for the natural path, provided t Q and ^ are not too far 
apart. 
The Lagrangean function : 



, ?m, ft, 
has the properties : 



(3) 2 



1,1 

is a positive definite quadratic form. Moreover, 

(4) H + L = J Pr q r , 

T 

where 

(5) Pr = J| r - 1, , m, 

and the Hamiltonian function 

H(q ly ,?,?!, -,pm, 
has the properties : 



* Oarathfodory has given a proof of this theorem : Riemann-Weber, Partielle 
Differenlialgleichungen der mathematischen Physik, 8. cd. 1930, Vol. I, Chap. V. 



382 MECHANICS 



A necessary condition that the integral (1) be a minimum is, that 



h 

8 fL 



8 I L dt = 0. 
The extremals are given by Kuler's equations : 



which are precisely Lagrange's equations. 

By the transformation (5), the inverse of which is given by 
(7), Lagrange's equations (8) go over into Hamilton's canonical 
equations, Chap. XI : 

dqr^M dpr___M r -i ... m 

(9) dt ~ dp r ' dt * dq r ' r ~ 1 ' ' m ' 
The latter can be solved by means of Jacobi's equation ; cf. Chap. 
XV and Appendix C : 

/im W . uf dv dv 

(10) _ + ff (, 1 ,...,, m ,_ ...,_ 

as follows. Let (q r Q , p r , t ) be a point in the neighborhood of 
which Equations (9) are to be solved. A solution of (10) : 

(11) V = S(q l9 - , q m , !,, , t), 
can be found * such that 



* * 
(12) - f ^ 

^(ll ' ' ' , ) 

* The existence theorem in question follows at onoo from the theory of character^ 
istics as applied to Equation (10). That theory tells us thut there exists a solution 
of (10) : 

V -Stai, -, Q m , 0, 
such that, when t = to, S reduces to a given function ^ (71, , Qm) : 

S (qi, - -, q n , to) - <f> (qi, , q m ). 

Here, <p (q\, , q m ) is any function which, together with its first derivatives, is 
continuous in the neighborhood of the point (qi, , q m ). Such a function is: 

<P (Ql, ' ' '. Qm) = Sr7r, 

r 

where the oti, , are m arbitrary constants, or parameters. The function *S 
thus resulting is the function required in the text. 

If, as we may assume, the function // (q r , p r , is analytic in the point (q r , 
p r , Jo), and if, as is here the case, <f> (q r ) is analytic in the point (g r ), then the 
fundamental existence theorem of the classical Cauchy Problem, formulated for the 
simplest case, applies at once, and the theory of characteristics is not needed. 



HAMILTON'S PRINCIPLE. LEAST ACTION 383 

in the point (q r Q , <*r, t Q ) and furthermore the equations : 

/-<o\ SS ~ 8S t 

(13) pr = Wf , fir -^, r = l,.-.,m 

are satisfied the first set, when (qv, p r , J ) are given, by the 
values a r = a r ; and then the second set determines /3 r . 

By means of this function S Equations (9) are solved. The 
solution is contained in (13) and is obtained explicitly by solving 
(13) for q r , p r : 



( . f ?r = /r(i, , m, ft, ' , ftn, 

I p r = grfai, ' ' ' , OW, ft, ' ' ' , j8m, 



t) 



Properties of the Extremals. If r/ r = </ r (0 represents an 
extremal, and if q r = dq r /dt, then by (5) and (13) : 

05) ^ r = ^ f , r = l, .-.,n. 

Moreover : 

(16) 2) 'M' + & = 

r 

For, since S is a solution of (10), it follows, by the aid of (13), that 

(17) S t + H(q l9 ,?,?!, ,p*,0 =0. 

On substituting this value of H in (4), and replacing p r in the 
resulting equation by its value from (13), Equation (16) results. 
The Function E(q r , q' T , q r , t). Consider the function 
V = L(q r ,q' r ,t), 

where (</ r , </J, t) are 2n + 1 independent variables. Let (q r , q r , 
be an arbitrary point, and develop L' about this point by Taylor's 
Theorem with a Remainder. We have : 

(18) V = L + 2) L ir (q' r - q r ) + E(q r , & g r , 0, 

r 

where L, Lq r are formed for the arguments (q ri q r , t), and 

(19) E(q r , Qr, <jr, = i 2 l iri , (q'r - q r M - ?.) 

r, s 

the coefficient I^ r Q 8 being the value of L<j r ^ for a mean value of 
the arguments q r , namely, q r + 0(q' r q r ), where < 8 < 1. 
The quadratic form (3) is positive definite. Hence 



384 MECHANICS 

(20) 0<E(q r ,q' r ,q r ,t) 

if (q'i, > m) is distinct from (ft, , g m ). 

Proof of the Minimum Property. Consider an arbitrary extremal 
(O Q through the point P : (q r , t<>), represented by (14) : 

: Qr = q r (t), r = 1, - , m. 

Let P! : (q r l , t\) be a second point on <~ near by. Connect P 
and P! by an arbitrary curve 

C: q r = q r (t), r = 1, , m, 

and let q' r (t) = dq r /dt. The curve C shall, however, be a weak 
variation, 

l?r(0-tfr| <>7, 

Let 

L = L(q r ,q' r ,t). 

Let (<?r, be an arbitrary point on C. Through this point 
there passes an m-parameter family of extremals, (13) or (14). 
We select one of them as follows. Let a lt , a m retain the 
values they have for <~ ; but let ft, , ftn have new values, 
namely, those given by the second of the equations (13), when 
q r = q r) i = t. The corresponding value of q r will be given 
by (7). It is the value found, for the a r , $ r in question, by dif- 
ferentiating the first of the equations (14) with respect to t. These 
values of r , q n q r , t satisfy Equations (15) and (16); the p r do 
not enter explicitly in these equations, and so the fact that they 
depend on t does not complicate the equations. 

We now apply Equation (18), setting q r = q r , giving to q r 
the value just found, and letting q' r refer to C, <f r = q' r . Thus 



(21) L = L(q r , q r , t) + % L^ r (q rj q ry t)(q' r - q r ) + E(q r , q'r, q r , 0- 

r 

The first two terms on the right of (21) can be modified as 
follows. First, 



(22) ^^ = S , r (q r , f)q' r + S t (q r , t). 
Next, from (16) : 

(23) 2 s , W" 9r + S, ($ - L (g r , (/ = 0. 

r 



HAMILTON'S PRINCIPLE. LEAST ACTION 385 
Subtracting (23) from (22) we have : 

^jj^ = 2) S, r (q r , t)(q' r - qj + L(q r , q r> f). 
Finally, since from (15) 



the first two terms on the right of (21) have the value dS(q r , t)/dt, 
and (21) can be written : 



(24) L = - + E(q r , q' n q r , f). 

We now proceed to integrate this equation from t to t v Ob- 
serve that 



to 

has precisely the value of the integral : 



ti 

CL <u, 



taken along the natural path of the system. For, along <~ Equa- 
tion (16) says that 

r> Q 
~ 



and so 

ti 

t. 



/Lett = 5fa r ,0 



to 



But in the end points, q r (t) = g r (0- We thus arrive at the final 
result : 



(25) 



i i 

CL dt = /L dt + CE(q r , $, q r , t) dt. 

to to o 



If, then, C differs from cF , there will be points of C at which 
E > 0, and so the integral of L over C (i.e. the integral on the 
left) will be greater than the integral of L over (" (i.e. the first 
integral on the right) and our theorem is proved. 



386 MECHANICS 

13. Jacobi's Integral a Minimum in a Restricted Region. In 

Jacobi's Integral : 

(1) 




the functions T and 'U do not contain t explicitly, and T is homo- 
geneous in the q r : 

(2) T= 

The varied functions, q r (u, ), are arbitrary, subject merely to 
the condition that dq r in each end-point, t t , t^ It is 
obvious that the integral (1) lias the same value as the integral : 



r t 
(3) JTdt, 



subject to the restriction : 

(4) T = U + h. 

This condition shall hold for the varied paths, too. Thus q r (u, c) 
is still arbitrary; but t(u, c) is determined by (4). To prove, 
then, that the integral (1) is a minimum for the natural path, it 
is sufficient to show that the integral (3) has this property, if 

(4) holds for the varied paths. 
In the present case, 

(5) L = T + U. 

(6) H = T - U. 
From (4) and (5), 

(7) L = 2T - h. 

Let (n Q be the path defined in 12, and let C' : 

(8) r = 7r(w, 0> ?=<(",), 

be a varied path. Consider the varied integral. From (7) 

t\ *i 

(9) /2? dl = fl dt + h(t l - * ), 



HAMILTON'S PRINCIPLE. LEAST ACTION 387 
where 



The right-hand side of Equation (9) can be computed as follows. 
From the analysis used in 12, Equation (24), we see that 

Li' 

du 
Hence 



Ldt = S(q r , I) "' + CEdl 
<b 



Since q r = q r for u = w , MJ, the first term on the right has the 
value : 

StorSZD-StorVo)- 
Hence 

* *i 

(10) /2T df = S fer 1 , ?i) - S far , o) + h (t, - t ) + CE dl 

to to 

Since // is independent of t : 



it follows as in Chap. XIV, 4, that a function S of the form : 
S = - ht + W(q l9 -,?*, A, 2 , -, a*) 

can be found, where h is to be identified with a v Using this 
function S in (10), we have : 



(11) ArdT = I^to, 1 ) - Fto r ) + Csdl 

<0 <0 

If we allow C" to coincide with <" , then J? ^ 0, and 

t\ 
J*2T<lt = W(q r 1 ) - W(q r ). 



388 MECHANICS 

Thus (11) becomes: 



C2Tdt = C2Tdt 

to t 



This proves the theorem. For, if C" is distinct from co'o, then 
J5, which is never negative, will be positive for some parts of the 
interval of integration, and hence the integral (3), extended over 
C', will exceed in value the same integral extended over the 
natural path, as was to be proved. 

The case U = const, leads to the geodesies on a manifold for 
which the differential of arc is given by the equation : 

ds 2 = 5} A rs dq t dq y . 

r, s 

Thiis we have a proof that a geodesic on a manifold obtained ar 
above is the shortest line connecting two points which are not too 
far apart. 



CHAPTER XIV 
CONTACT TRANSFORMATIONS 

1. Purpose of the Chapter.* The final problem before us is 
the integration of Hamilton's Canonical Equations : 

.. dq r 8H dp r 8H , 

A) df = Wr' dT = -W,' r=l '-' m - 

The method consists in finding a large and important class of 
transformations of the variables (q r , p ry t) into new variables 
(q' r , p' r , t'), such that Equations A) are carried over into a new 
system of like form : 

A/ , dq' r 3H' dpr 3H' t 

A) W = W dr = ~W r - 1 '-' w ' 

or, as we say, transformations with respect to which Hamilton's 
Equations remain invariant. 

The most general class of such transformations we shall con- 
sider, are the so-called Canonical Transformations. A one-to-one 
transformation : 



<lr = qr(q ly ' -,7m, 


Pi, ' 


, Pm, 


Pr = P' (ft, ' ' ' , (7m, 


Pli ' ' 


' , Pm, 


f = ' (ft, -,?, 


Pi, * * 


' , Pm, 


(ft', ' "^m. Pi', " 


* , Pm, 


O^n 



01, ' ' ' , tfm, Pi, ' ' ' , Pm, 

is said to be canonical if there exist two functions, 

H(<li, ' ' , 7m, Pi, , Pm, and H' (q(, - , q' m , p(, , Pm, t') 

(not in general equal to each other) such that 

* This introductory paragraph is designed to give an outline of the treatment 
contained in the following chapter. The student should read it carefully, not, 
however, expecting to comprehend its full meaning, but rather regarding it as a 
guide, to which, in his study of the detailed developments, he will turn back time 
and again for purposes of orientation. 

389 



390 MECHANICS 

(1) /(2 V'M - H'df) = J(2 Prdqr - Hdt), 

1" 1' 

where F is an arbitrary closed curve of the (2m + l)-dimensional 
(gv, ?>r, 0- s P a( ' > ail( l V' * s its image in the transformed (#J, pj, <')- 
space, these spaces being thought of as simply connected. 
To a canonical transformation there corresponds a function 

' ' ' i <7m, Pi, - , Pm, such that 



(2) 2 ?' M * H ' dt ' = ^ Prdq r - Hdt 



And conversely, when three functions H', H, ^ exist, for which 
the latter relation is true, the transformation is canonical. 

Contact Transformations. An important sub-set of these ca- 
nonical transformations consists in those for which the last Equa- 
tion I. is 
(3) f = t. 

On equating the coefficients of dt on the two sides of Equation (2) 
we find : 

' 



Since /' = /, we may say that the variable t is not transformed, 
and treat it as a parameter. Equations I. thus take on the form : 



with 



<?' = q'rfal, ' ' ' iQmiPi, ' ' , Pm, t) 
Pr = Pr(q\y ' ' ' , Qm, Pi, ' , Pm, t) 

^(<7?> <?m, P' } , ' ' 9 Pm) _^ 
d(9l9 ' ' ' , (7m, Pi, ' ' ' , Pm) 



And now comes an important modification of Equation (2). 
Since we now are regarding the (q rj p r ), and not the (q r , p r , t), 
as the independent variables, (2) can be written by the aid of 

(4) in the form : 

(5) %(p'dq' r - p r dq r ) =d*. 

r 

Of course, d$ has different meanings in (2) and (5). In (2), 

^\ ^T, 

(6) l 



CONTACT TRANSFORMATIONS 391 

since here the independent variables are q r , p r , t, whereas in (5), 

/*\ JT 

(7) * 



since here the independent variables are g r , p r ; a similar remark 
applying to the other differentials, dq' r . This is not an exception, 
or contradiction, in principle, but only in practice, since the 
differential of any function, *(i, , x n ), depends on the inde- 
pendent variables : 

__ ^ <Nf 

and it is not until we have said what these shall be i.e. defined 
our function that we can speak of its differential. 

A transformation we will henceforth change the notation 
from m to n : 

( , f Qr = ?'(<?!, ' ' ' , 9n, Pi, ' ' ' , Pn) 

I Pr = Pifei, ' ' ' , tfn, Pi, ' ' ' , Pn) 

3 (ft', ' ' ' , 0i> Pl' ' ' ' , Pn) , n 



#ft> ' ' ' , 0n, Pi, ' ' ' , P 

such that 

(9) Jpfdtf = jprdq r , 
r' r 

where F is an arbitrary closed curve of the (QV, p r )-space, thought 
of as simply connected, and F' is. the curve into which it is trans- 
formed, shall be called a contact transformation. There cor- 
responds to such a transformation a function ^(q lt , q nj 
Pi> ' ' > Pn) for which 

(10) 2,(prdq' r -prdq r ) = d*. 

r 

And conversely, a transformation (8) for which (10) is true satis- 
fies (9) and so is a contact transformation. 

A contact transformation may, of course, depend on certain 
parameters, p', q' r and thus becoming functions of these para- 
meters as well. The transformation II. above is a case in point. 

Finally, the canonical transformations form a group; i.e. the 
result of applying first one and then a second such transfor- 
mation may itself be expressed as a canonical transformation. 



392 MECHANICS 

The contact transformations also form a group. The group of 
contact transformations II. is a subgroup of the group of canonical 
transformations I. 

The approach to the contact transformations is through the 
Integral Invariants of Poincarg. 

The contact transformations, as defined generally by (8) and 
(9), are of especial importance in Mechanics because any such 
transformation carries an arbitrary system A) of Hamiltonian 
Equations over into a second such system, A') ; cf. infra, 4. 
We shall treat the application of these transformations to the 
integration of Hamilton's Equations at length in Chapter XV. 
If the student is willing to take this one property of contact 
transformations for granted, he can turn at once to Chapter XV, 
and he will find no other assumptions needed in the study of 
thajt chapter. 

2. Integral Invariants. Consider the action integral : 

*i 

(1) j*L(q r ,q' n {)dt, 

to 

and the extremals, which are the path curves, given by Lagrange's 
Equations : 

/o\ ^ **L ^ _ n 1 

(2) diWr Wr~ ' r-V-.,n, 

where L is the Lagrangean function, or the kinetic potential. 
The general solution can be written in the form : 

(3) q r = q r (t ; qf, , qJ, qf, , tf n ), r = 1, , n, 

where g r , q r are the initial values of q r , q r , i.e. their values 
when t = fo. In the (2n + l)-dimensional space of the variables 
(<7u * ' * 9 q*> <ii> * ' ' > q*9 these equations, together with the n 
further equations : 

(4) <?r = <?r('; 1, ,?, ?1, ,<7n)> 

represent a curve C, or more properly, a 2n-parameter family 
of curves C. Let a closed curve, F : 

(5) ?r = ?r(X), tf r = g r (X), r = l, , n, X S X g X,, 

be drawn in the plane t = . The curves C which pass through 
the points of F form a tube of solutions, which we will denote by S. 



CONTACT TRANSFORMATIONS 



393 



Let the action integral, (1), be extended along the curves C 
which form S. Its value is a function of X : 



(6) 



where q r , q r are given by (3) 
and (4) and q r , q r by (5). 
Differentiate / (X) : 




FIG. 147 



- C 

" J 



On integrating by parts, observing that 



we have : 
Hence 



d dq r 
di~d\' 



C'^^LM = 3L<^- C^^^SLM 

J d</r 3\ d(j r 3\ J dtdq r 3\ 

t\ 

'(\\ - C V (^ J d 3L\ fyr,, | y dL8q r 

() ~ J $ \Wr dtWr' 8\ CU + -f 2q r d\ 



The integral vanishes, because q r is by hypothesis a solution 
of (2). 

We now make the transformation, Chapter XI, 3 : 



(7) 

Thus 

(8) 



dL 



Since F is a closed curve, q r (\) = ^r( 
and (6) gives : 

(9) 
Hence 



X 



0, 



394 MECHANICS 

and so from (8) : 

*i 

/ k P/y <l 

eJX = 0. 



Let t be thought of as constant, but t l9 which is also arbitrary, 
as variable ; denote the latter by t. Then 



This equation represents the theorem in which the whole in- 
vestigation of this paragraph culminates. In substance it can 
be stated as follows. We may regard Equation (7), along with 
the n + 1 further identical equations, q r = q r , t = t, as repre- 
senting a transformation of the (q r , q r , )-space on the (q r , p rj 0" 
space. Observe that the Jacobian 

- ?j 





Chapter XI, 3. Thus the curves C of the first space go over 
into curves C" of the second space, and F goes over into a curve 
TO, S being transformed into a tube S'. 

Let us now make the second space the space of the vari- 
ables (<?r, p r , t) our point of departure and, dropping the primes, 
consider a closed curve in the plane t = t Q of that space : 



Consider furthermore curves C through its points, which are 
obtained by transforming the curves C of the earlier space. The 
integrals (11) now become line integrals in the present space. 
If we change the notation, setting 

(13) q r Q = r, Pr = Pr, 

then (11) assumes the form : 



(14) 



/5J Prdq r = / ^0rda r , 
r *J r 



where F is the curve of intersection of the arbitrary plane / = t 
with the tube S determined by T , an arbitrary closed curve of 



CONTACT TRANSFORMATIONS 



395 



the plane t = t Q . But this is precisely the definition of a contact 
transformation, t being thought of as a parameter : * 



, . 



Pr(i, 



, , ft, 

' i n , ft, 



, fti, 



3. Consequences of the Theorem, a) Hamilton's Canonical 
Equations. Lagrange's Equations (2), 2 form a system of n 
simultaneous total differential equations of the second order. 
By means of the transformation (7) these are carried over into 
a simultaneous system of 2n total differential equations of the 
first order in the (q r , p rj 0-space. Let these be written in the 
form : 

(16) = Qrfop,0, Pr(?,P,0, 



Since the right-hand side of (14) is independent of t, the deriva- 
tive of the left-hand side with respect to t must vanish. Hence ' 



or 



*1 

d C ^-\ dq r j\ _ (\ 

dij 2,P'^ dX - u ' 
?1T a\ r + pr aTax) dx = ' 



Integrate by parts : 



d\ 



n 

pr 



Since T is a closed curve, 



= 0, 



*The geometric picture is here slightly different from the earlier one, since 
the variables (a ri /3 r ) and (q rt p r ) are interpreted in different planes. But of course 
one may think of a cylinder on T as directrix, with its elements parallel to the 
t-axis. On cutting this cylinder with the plane t = t, we have a curve F lying in 
the same plane with F. Or, to look at the situation from another angle, t is only 
a parameter, and it is the spaces of (a r , Pr) and (q r , p r ) which concern us. 



396 MECHANICS 

and we have : 



Here, 

dq r __ dqr _ n tyr __ dp r _ p 

8t ~ dt ~ Wr> dt ~ dt " 

Thus Equation (17) may be written in the form : 

(Prd r -Q r d r ) = 0. 



But r may be any closed curve of the plane t = /, since to any 
such curve in that plane corresponds a F in the plane t = t . 

It follows, then, that we can define a function // by moans of 
the integral : 



, 
(19) H = f -Prdqr 

' 



where the fixed point (a lt , a n , b lf , &, ) of the plane t = t 
is connected with the variable point (q ly , q ni Pi, , p n , 
of this same plane by a curve lying in the plane. Because of 
(18) the value of the integral does not depend on the path, 
and thus // is defined as a function of (q r , p r ) for the particular 
value of t. 

Let the point (a, &, t), for dofinitcness, lie on the extremal through 
the point (a, 0', 2 ). Then H becomes a function of (q rj p r , 0- 
If (c/, 0', J ) is replaced by a different point (a", /3", t Q ), the 
new H will differ from the old H by an additive term which is a 
function of t, but not of (q r , p r ). 

More generally, let // be defined by the equation : 

(20) II = li+f(i), 

where H is a specific one of the functions 77 just defined, and 
f(t) is an arbitrary function of / alone. 
From (19) it follows that 

dn 



CONTACT TRANSFORMATIONS 397 

Thus the system of equations (16) is seen to have the form : 

, , dg r _SH dp r _ 8H 

(22) Hf-Wr' ~dt~~Wr' r=l,. ..,n. 

First fruits of our theorem. The Hamiltonian Function H 
grows naturally out of Equation (14) ; for (18) is but another 
form of (14), and (18) at once suggests the definition of // by 
(J 9) and (20). Thus if we had never heard of H through the trans- 
formations of Chapter XI, we should still be led to it by the 
theorem of this paragraph. 

The Function V and Its Relation to H. Equation (14) can be 
written in the form : 



f 

To 



lr- Prdctr) =0, 



where g r , p r are given by (15), the curve F being as before any 
closed curve in the plane t = t . It follows, then, that the integral : 

(<*,$) 
(23) 



extended over an arbitrary path in the plane t = t joining the 
points (a', jft'), (a, /?), is independent of the path and thus 
defines a function of (a, 0), t entering as a parameter : 

(J5) 
(24) g (Prdqr - Prdctr) = V (<*, ft t). 



f 

('>) ' 



Differentiate this equation with respect to / : 






dq r \ __ dV 

'~ 



where the italic d means differentiation along a curve (15). Trans- 
forming through integration by parts we have : 

/o c x rj r , dv 

(25) 



r 



_ 



398 MECHANICS 

The integral^ on the left is precisely the negative of the integral 
(19), or H(q r , p r , f). Hence 

(26) H = 2 PrQr ~ ^, 

where H is given by (20), and 



On the other hand, the Lagrangean Function L (q r , q r , t) is 
connected with H (q r , p r , t) by the relation (cf . Chapter XI, 3) : 

(27) L + H = ]T p r q r . 

r 

Hence it appears that 

<*> - - 

Just as H was defined only save as to an additive function of t, 
so V can be modified by adding any function t y and the same 
is true of L. But it is convenient to restrict these additive func- 
tions so that (26) and (27) will hold. 

From the foregoing reasoning we can draw a more general con- 
clusion, and then supplement it with a converse. 

THEOREM I. Let 



r = l,---, n, 

be an arbitrary system of simultaneous differential equations t and let 
q r = <p r (t ; !,--, or n , ft, , j9) 

be the solution, where a r , Pr mean the initial values of q r , p r cor- 
responding to t t . Let TQ be an arbitrary closed curve lying 
in the plane t = t Q of the (2n + l)-dimensional space of the vari- 
ables (q r , p r , t). Let S be a tube consisting of the curves ii) which 
pass through points of F ; and let T be the section of S by the plane 

-. // 

Pr dq r 



\ 5) 



CONTACT TRANSFORMATIONS 399 

is an integral invariant of Equations i) ; i.e. if 

iv) I ^Prdq r = I ^LfPrdotr, 

r ' r 

then Equations i) form a Hamiltonian System: 
. dq r dH dp r dH , 

i -/*_ = . r . = r = 1 ti 

"' dt 8p r ' dt 8q r > T lf >n ' 

Conversely, if Equations i) form a Hamiltonian System y), then 
Hi) will be an integral invariant, or iv) mil be satisfied. 

Observe, however, that Theorem I. is more general than its 
origin from the action integral (1) and the transformation (7) 
would indicate. It applies to any functions Q r , P r for which 
Hi) is an integral invariant ; or, in the converse, to any function 
H, provided that the determinant 

02 TI 
H u ".H nn * 0, H i3 = - 



But a system of Equations v) may conceivably not lead to a 
mechanical problem why should it ? 

b) Contact Transformations. The content of Theorem L can 
be restated in terms of contact transformations. 

THEOREM II. Let 

qr 9r( a D ' ' ' , <*n, ft, ' * ' , ft, t) 



a) 

hr(ot lt ' ' ' , n, ft, ' ' ' , fti, 

where r = 1, , n, 

Pi, 



0^, -,., ft, --^ftr ' 

a?id 

f a r = gfrC^, , a n , ft, , ft, < ) 

I ^ r = A r (a!, , a n , ft, ' , ft, O 

fee a transformation of the 2n-dimensional (<x r , p r ) -space on the 
(q r , p r )-space; and let 



400 MECHANICS 

be the system of differential equations corresponding to a) ; i.e. 
defined by a). // a) is a contact transformation; i.e. if 



I ^Prdq r = j ^Prdar, 



or 



2J (p r dq r - Prdoir) = dV (a, /3, /), 

r 

then b) z's a Hamiltonian System: 

C ' ~dt ^ ~dp~ r ' ~dt = '"~ ~dq r ' r== >'"> n > 

and conversely. 

4. Transformation of Hamilton's Equations by Contact Trans- 
formations. If we start out with a given system of Hamiltonian 
Equations : 

, , dqr _ dH dpr dH_ __ 1 

() ~dt ~ 8p~ r ' ~dt " ~dq~ r ' r-I,---,n, 

and make an arbitrary transformation : 

/0 , f 9r = /rfe, ' ' ' , ^n, Pi, ' , Pn, 

W 1 , , A 

I Pr = Vr(q\y ' ' ' , ?n, Pi, ' ' ' , Pn, 



the transformed equations : 
(3) 



r = 1, , n, will not in general be of the form (1) ; i.e. they 
will not have the form : 



where /f ' = H' (q' T , p' r t) is some function of the arguments q' T , p' r L 
A sufficient condition that (3) be Hamiltonian, i.e. of the form 
(4), is that (2) be a contact transformation. 

The proof is based on Theorem II., 3 and the fact that the 
contact transformations form a group. Let (2), then, be a contact 
transformation. Denote it by T. Let (aj, #) be the initial val- 



CONTACT TRANSFORMATIONS 401 

ues of (?', p'r) for t = t Q . They arise from (a r , r ) by T, formed for 
* = *o J ^o> let us write it. Thus, symbolically, 

(*;, #) = T (a r , r ), or ( r , r ) = T Q -*(cl, ft). 
Again, we may write symbolically : 

(#, PJ) = T (g r , p r ). 

Finally, consider the solution of (1), whereby the space of the 
(a r , p r ) is carried over into the space of the (g r , p r ). This 
transformation is the Transformation a) of Theorem II. , 3, and 
so because of (1) is a contact transformation. Denote it by D : 

D ( r , r ) = (q r , p r ). 

On the other hand, the effect of the transformation defined by 
the differential equations (3) is to carry the space of the (a' Ty ft) 
over into the space of the (q' r , p r ). Denote it by A : 



And now we see that this result this transformation A can 
be obtained as follows : Perform first the contact transformation* 
TQ I on the (aj, $)-space, thus obtaining the (a r , /3 r )-space : 

(a r , 0J = 57 (;, #) 

Next, perform the contact transformation D on the (a r , fi r )- 
space, thus obtaining the (q r , p r )-space : 



Finally, perform the contact transformation T on the latter space, 
thus obtaining the (q' r , p'J 



fer', Pr) = T (q r , p r ) 

We have in this way obtained A as the result of three contact 
transformations : 

A = TDT?. 

Hence A is itself a contact transformation, and so the system (3) 
is Hamiltonian, by Theorem II., 3. 

This is the result on which the developments of Chapter XV 
depend. It may be stated as follows. 

* The inverse of a contact transformation is obviously itself a contact transfor- 
mation. 



402 MECHANICS 

THEOREM. // a system of Hamiltonian Equations (1) be trans- 
formed by a contact transformation (2), the result is a Hamiltonian 
system (4). The condition is sufficient, but not necessary. 

Computation of H'. The original system of Hamiltonian 
Equations (1) leads to the contact transformation Z), for which 
the relation : 



(5) ^ p r dq r - 2 ^ dar = dV (a ri r , t), 

r r 

is characteristic, where 

JT "V /n A __ 

dt 



(6) 77 = 2 Prtfr - ~ 



The transformed Hamiltonian Equations (4) lead likewise to 
a contact transformation D' = A, for which the relation 



(7) 2 P' M - 2 # da ' = dV> ('. '> 

r r 

is characteristic, where 

j jr/ 

Let 

r r 

be the characteristic relation of the contact transformation T. 
Then 

(10) 2 # da ' " S ^ dc * r = dW (<*" & r > *o) 

r r 

will be the characteristic relation corresponding to T . 

Each of the differentials on the right is taken on the supposi- 
tion that t is a parameter, and so a constant. Moreover, (q r> p r ) 
are given in terms of (a r , Pr) by equations of the type a), 3. 

From (5), (9), (10) we infer that 

r r 

d[- W(ct r , ftr, < ) + V(a r , 0r, H 



CONTACT TRANSFORMATIONS 403 

Hence 



- 

dt ~ dt dt' 

provided V (a r , $, f) and W(q r , p r , 0, which arc determined only 
save as to additive functions of t, are chosen properly. From 
(6) and (8) we now infer, by means of (12), that 



(13) H' = H - + (p'^ - p r q r ). 

Each of the functions H', H, dW/dt was originally defined 
only save as to an additive function of t, and it is only when 
these additive functions are suitably restricted, that (13) holds. 

6. Particular Contact Transformations. In applying the theory 
we have developed it will be convenient to denote the trans- 
formed variables by Q rj P r instead of by q' n p' r . Thus a trans- 
formation : 

f Qr = /rfoi, , <7, Pi, , p, 

I P r = <7r(<7i, - ' , Qn, Piy ' ' , Pn, 

where 

' , (jft, 1 l)'*'? * n) ^ Q 
' " * ' ' 



is a contact transformation if 

(3) 2 (P r dQ r - Pr .rf7r) = ^^ (<7r, Pr, 0, 

r 

where is regarded as a parameter and the differentials are taken 
with respect to (q r , p r ) as the independent variables. 

If such a transformation be applied to the Hamiltonian system : 

(4\ dqr__<M ^Pr__^ff -_!... 

W dt dp r ' dt dq r ' lj ' n ' 

these equations go over into a new Hamiltonian system : 

dQ,_ff' dPr__W _j ... _ 

W <tt ~ P,' rf< ~ 3Q,' ' ' ' 

where H' (Q r , P r) is connected with H (q r , p r , t) by Equation 
(13), 4, or: 

(6) H' = H - + (P r Q r - p r q r ). 



404 MECHANICS 

The (q r , Q r , t) as Independent Variables. Equations (1) repre- 
sent 2n relations between the 4n variables (g r , p rj Q r , P r ), and 
when (q r , p r ) are chosen as the independent variables, (2) and 
(3) hold. It may be possible to choose the 2n variables (q rj Q r ) 
as the independent variables, t always being regarded as a para- 
meter in (3). Write 

(7) W(q r ,pr,t) = W'(q r ,Qr,t). 
Thus (3) becomes : 

(8) 5 (PrdQr - PrdQr) = dW (q r , Q r , t) . 



On equating the coefficients of dQ r , dq, in (8) we find: 

P r = 

(9) 



Equation (6) can now be transformed as follows : Since 

dW dW dW'dQr SW'dq r 8W 

' 



dt dt 'dQ r dt ? 8q r dt dt ' 

we have : 



Hence (6) becomes : 

(10) ff ' - ff - 



OO OO 

The Transformation: p r = -^-, P r = ^T' We can write 

Oq r Glflr 

down a particular contact transformation, in which (q r , Qr) can 
be taken as the independent variables. Let 



' , q n , !, - , a ny t) 
be a function of the 2n + 1 arguments such that 



CONTACT TRANSFORMATIONS 405 

Set a r = Qr and make the transformation : 

/irk\ &S r> &S i 

(12) Pr = Wr , Pr=~ Wr , r = l,...,n. 

The first n of these equations can be solved for the Q r in terms 
of the (q r , p r ) because of (11), and then the P r are given by the 
last n equations. Thus a transformation (1) results, the Jacobian 
(2) not vanishing.* 
The transformation will be a contact transformation, for 



(PrdQ r ~ Pr dq r ) = ~ (|| dQ r + J dq r ) = ~ d3, 

and we may set W = S, since Tf and hence FT' is determined 
only save as to an additive function of t. Equation (10) now 
becomes : 

(13) H' = H + - 



How such a function S can be found, which will enable us to 
solve Hamilton's equations explicitly, will be shown in Chapter 
XV. 

Conversely, the most general contact transformation (1) which 
can be written in the form : 



is given by (12). For, Equations (9) must be true, and it remains 
only to set S W. It is seen at once that the W r of (9) must 
satisfy (11), since otherwise there would be a relation between 
the P r . 

* The proof is as follows. If 

Vr = fr (Xl, -, Xn), T = 1, , U, 

be a transformation having an inverse 

Xr = V ? r (l/Ii ' ', 2/n), f = 1, , n, 

where f r , <f> r are all functions having continuous first derivatives, then 

d (y\, - -, yn) . d (x\, , x n ) _ j 

d(xi, - -,*) d(yi,--,yn) 
Consequently neither Jacobian can vanish. 

In the present case, the q r , Pr can be expressed in terms of the Q r , P r , since the 
value of the determinant (11) is unchanged if the q r , a r are interchanged. 



406 MECHANICS 

EXERCISES 

OO ^Cf 

1. The Transformation: p r = T , Q r = ^p- Study the 

oq r Of r 

analogous case, in which (q r , P r ) can be taken as the indepen- 
dent variables, t being, as usual, a parameter. Show that, if 
(#u ' > Qn> <*i> ' * * > <*n, be chosen as before, and if we set 
P r = a r , then 

/-. ^\ v*S s^ O& - 

(14) p, = w , Qr= W , r = l,..-,n, 

will give a contact transformation. Observe that (3) can be 
transformed by means of the identity 

d(P r Q r ) = PrdQr + QrdPr, 

so that it takes on the equivalent form : 

rdPr + prdq r ) = d(~ W" + P r Qr). 



Choose W(q r , p r , = W"(q r , I\, t), therefore, -so that 
S=- W" 



Compute dW"/dt and show by the aid of (14) that (6) yields : 
(15) ff' = // + . 

State also, and prove, the converse. 

2. Computation of //' in the General Case. Let TT^ , 7T 2ri 
be any set of 2n variables, chosen from the 4n variables 
far, Pry Qr, Pr), in terms of which the remaining 2n variables 
can be expressed. Show that 



06) -, 

where q r , Q r , and W are expressed as functions of (TT*, 0- 

/)^f OC| 

3. The Transformation : q r = -5 , P r = -^r- If (p r , Qr) can 

Gpr #V r 

be taken as the independent variables, and if we set 

S = W + Pr?r, 



CONTACT TRANSFORMATIONS 



407 



where q r , W, and S are now functions of (p r , Q r , t), then the 
transformation takes the form : 



(17) 

and (6) yields : 

(18) 



= _ 

^ d P r' ' 



H' = H - 



Conversely, if S(q lt , q n , a lt , a n ) be chosen as before, and 
if we set Q r = QL r , then (17) will define a contact transformation. 

6. The fi-Relations. There is one case of importance still 
to be considered, namely, that in which W is a function of 
(q r , Qr, t), but the (q rj Q r , t) cannot be chosen as the independ- 
ent variables. The extreme case would be that in which 



Qr = Wr 



T = 



n, 



Tho general case is that in which < m ^ n independent rela- 
tions between the (q r , Q r , t) exist, and no more : 

where the rank of the matrix : 

X^ Xli 



(2) 



Wn 



is m. Thus m of the Q*'s can be expressed as functions of the 
remaining ju = n m Q/s and q^ , q n , t. As a matter of 
notation let the above m Q fc 's be Q D , Q m : 

/O\ /") ___ / ' f\ f\ n ff /\ __ 1 /yyj 

Then the determinant whose matrix consists of the first m columns 
of (2) will not vanish. Among the 2n (p r , P r ) it shall be possible 
to choose m variables, TTJ, , w m such that (ir lt , 7r m , Q m +i, 
* ' ' > Qn, <7i, , ^n, can serve as the 2n + 1 independent 



408 MECHANICS 

variables. But the function W(q r , p r , t), when expressed in 
terms of the new variables, does not depend on ir ly , ir m : 

(4) W(q f , Pr ,t) = IF* for, Or, fl. 

It is not, of course, unique, because of the Q-relations, (1). 
Equation (3), 5 now takes on the form : 

(5) 2) ( Pr dQ r - p r cfy r ) = dW* (q r , Q r , 0. 
We will rewrite it in the form : 



I (^-CK -?(* 



It is not, however, in general true that the coefficients of the 
differentials vanish. 

By means of the m equations (1) the first m differentials 
dQu , dQ m can be eliminated, the resulting equation being 
of the form : 

(7) X m+l dQ m +t + + XndQn + Y.dq, + - - + Y n dq n = 0. 

The differentials in (7) are independent variables, and so we can 
infer that 

X m+l = 0, - . , X n = 0, Y, - 0, , Y n = 0. 

The actual elimination can be conveniently performed by 
means of Lagrange's multipliers. From Equations (1) we infer 
that 



n 

n = o 



(8) 



Multiply the fc-th of these equations by X& and add to (6). Then 
determine the X/t's so that the coefficients of dQ } , , dQ m vanish. 
The resulting equation is of the form (7), and so its coefficients 
vanish automatically. We thus arrive at the 2n equations : 



(9) 



_ 

' ~ Wr + ' Wr 



r = l ... m 



CONTACT TRANSFORMATIONS 409 

The first m of these equations determine the \ k 's. The remainder 
are satisfied as shown above. The result is symmetric and holds, 
no matter what set of m Q k 's is determined by (1) ; i.e. no matter 
what ?n-rowed determinant out of the matrix (2) is different 
from 0. 

It is now easy to determine H f by means of (13), 4 : 



On replacing P r , p r here by their values from (9) and observing 

that 

dW* 



= 
dt d Q r dt , dQr d { dt > 

dtt r ^ dttr dQr . ^ d&r ^r , ^r ^ 

dt "" 2? 3Q r dt ^ ^ dq r dt ^ dt ' 
we find the following result : 



-- -J 

If, in particular, the 12's do not contain t explicitly, this equa- 
tion reduces to 

(11) H' = H 



CHAPTER XV 
SOLUTION OF HAMILTON'S EQUATIONS 

1. The Problem and Its Treatment. We have considered a 
great variety of problems in mechanics, the solution of which 
depends, or can be made to depend, on Hamilton's Canonical 
Equations : 

m dqr - dH dpr -- m r-1 ..- n 

(i) ~dt~~Wr' ~dt ~ Wr ' ' ' 

where H is a function of (q r , p r , ). The object of this chapter is 
to solve these equations explicitly in the important cases which 
arise in practice. 

The method is that of transformation. By means of a suitably 
chosen transformation : 

Qr = F r (q 19 , q n , Pi, , P, 

P r = G r (q ly ' - - , q n , Pi, ' ' , Pn, 

Equations (1) are carried over into equations of the same type : 



dt ~ d/V dt 



' 



but more easily solved. Here, H' is a function of (Q T , P r , <)> 11( >t 
in general equal to H . 

The determination of a convenient transformation (2) depends 
on a partial differential equation of the first order, due to Jaeobi * : 

(A\ dV _i_ 

(4) -- + 

It is not the theory of this equation, however, but the practice, 
that concerns us, for all we need is a single explicit solution, 

(5) V = V(q lf , g, i, , n, 0, 

depending in a suitable manner on n arbitrary constants, or 
parameters, !,-, n . Such a solution is found in practice by 
means of simple devices, notably that of separating the variables. 

* Hamilton came upon this equation ; but its use as here set forth is due to Jaeobi. 

110 



SOLUTION OF HAMILTON'S EQUATIONS 411 

The function (5) once found, the further work consists merely 
in differentiation and the solution of equations defining the 
q r , p r implicitly. Two cases are especially important, namely : 

a) Reduction to the Equilibrium Problem. Here, a solution 
(5) of (4) enables us so to choose (2) that the transformed H 
vanishes identically, //' = 0. Equations (3) can now be inte- 
grated at sight : 

where a r , ($ r are arbitrary constants. On substituting these val- 
ues in (2), the inverse transformation, 

f qr = /r(Q!, -,, PI, ,P,0 
yields the desired solution : 

q r = /r(i, ' ' ' , n, ft, ' ' i fti, 



(8) 

Pr = 0r(i, ' ' ' , <*, ft, ' ' ' , ft, 

The transformation (2) in this case, as will be shown in 2, is 
given by the equations : 

, . _ dV p _ dV _ t 

^ Pr ~Wr r ~~Wr' r-l,..-,^ 

where F is written for the arguments q r , Q r : 



Thus the solution (8) is obtained by solving the equations : 

dV dV 

pr = Wr' &T =~^ r=l,..-,n, 

where the present V has the form (5). 

b) Constant Energy, H (q r , p r ) h. The second case is that 
in which H does not contain the time explicitly : 

H = H(q l9 ,g, Pi, ,pn). 

It is here possible to find a transformation (2) in which F r , G> 
do not depend on t, 

Q r = F r (q lf , g w , p lf , p n ) 



(10) 

' ' ' , ^n, Pi, ' , 



412 MECHANICS 

such that the new H will depend only on the P rj but not on 
Q rj t. In particular, 

#' = P^ 

Equations (3) now take on the form : 



= 0, r=l,...,n. 
Thus* 

Qi = t + /3 } , Q, =ft, 5 = 2, 



P r = a r , r = 1, , n. 
Let the inverse of (10) be written : 

(12) 

Then the solution of (1) is given by the formula : 



(13) 

1 ft, ft, 

The transformation (2) in this case, as will be shown in 4, is 
given by the equations : 

HA\ dW n 

(14) pfSS Wr 9 Qr = 

where W is a solution of the equation : 

iff m dW 

^'-'^ 

or: 

Tf = W(q l9 ,?n, A, 2 , ,) 

Here TF depends on the arbitrary constant A, and also, in a suitable 
manner, on n 1 further constants, or parameters, a 2 " * ' t <** 
These are set equal respectively to the P r : 

Pi = h ; P, = a a , s = 2, , n. 

* The change of notation whereby the a/s and the /Vs are interchanged is made 
for the purpose of conforming to usage in the literature. 



SOLUTION OF HAMILTON'S EQUATIONS 413 
Equations (14), combined with (11), thus yield : 



(15) ,w 



The last n 1 of these equations can be solved for q^ , q n 
in terms of q ly as will be shown in 4, thus giving the form of the 
path ; and then q can be found from the first equation (15) in 
terms of t. 

We have characterized this case by the caption: "Constant 
Energy," but this is not a physical hypothesis. Our hypothesis 
is, that H does not depend explicitly on 2, and this is all we need 
for the mathematical development. That H then turns out to 
be constant along the curves of the natural path, is an impor- 
tant consequence; but our treatment does not depend on this 
hypothesis. 

Contact Transformations. The transformations used in a) and 
b), namely, (9) and (14), are examples of contact transformations. 
A transformation (2) with non-vanishing Jacobian was defined 
in Chapter XIV, 1, to be a contact transformation if 

(16) 2} (PrdQr - Prdq r ) = dW (q r , p r , t), 

r 

where the differentials are taken with respect to the (q r , p r ) as 
the independent variables, t being regarded as a parameter. Such 
a transformation always carries a Hamiltonian System (1) into 
a Hamiltonian System (3). That the transformations (9) and 
(14) satisfy the condition (16) is seen at once by substituting 
in (16), observing in the case of (14) that 

d(PrQr) = PrdQr + QrdP r . 

This is all the theory the student need know from Chapter XIV, 
to enter on the study of the present chapter, and this amount 
of theory was all developed in 1-4 of that chapter. 

2. Reduction to the Equilibrium Problem. We have seen in 
Chapter XIV, 5, that a transformation : 



414 MECHANICS 

where 

S = 8(q if -, fr, -, ) 

is any function such that 



and where Q r is set = a r , will carry the Hamiltonian System (1) 
of the last paragraph over into a Hamiltonian System (3), where 

(2) /r-ff + f. 

The transformed function H' can be made to vanish identically 
if we can find a solution V of the partial differential equation : 



which depends on n arbitrary constants, a ly , a n : 

V = V(q lJ , ?, !,-, a n , 0> 
and is such that 

^.......vj^ 

3(ll >) 

On setting S equal to this function F, and making the trans- 
formation (1), H' as now determined vanishes identically. Thus 
the transformation : 

(5) p, = g, Pr jfc r=l,...,n, 

where a r is replaced by Q r in F, transforms the Hamiltonian 
System (1) to the Equilibrium Problem: 

t-o- T'-- '- 1 '-'"' 

The solution of these equations is the system of equations (6), 
1. These are the values of Q r , P r to be substituted in the 
transformation (1) ; i.e. in the present case, in (5) : 

(7) p, = g, 0,=~g, r-l,... f . 

The last n of these equations can be solved for the q r 's because 
of (4), and then the first n equations give the p r . 



SOLUTION OF HAMILTON'S EQUATIONS 415 

There is, of course, a further requirement in the large, namely, 
that the a r , $r can be so determined as to correspond to the initial 
conditions : t = t Q , q r = q r Q , p r = Pr. Thus the equations : 

Pr = V r , - , g n , !,, n , Q, r = 1, - , n, 

must admit a solution, a r = a r , and V (ft, , q n , a l9 , e* n , 
must satisfy all the conditions of continuity, notably (4), in the 
neighborhood of the point (q r , a r ) = (<7r, a r ). 

EXERCISE 

Pass to the Equilibrium Problem by means of the transforma- 
tion studied in Chapter XIV, 5, Exercise 1 : 

dS n dS 1 

*'~W Qr = W r > " = V--,". 

Here, 



Let V = V(QI, , q n , a lf , a n , be the same function as 
that of tho text a solution of Equation (3). If, then, we 
replace a r by P r and set S = V, the transformed H ' will vanish : 
//' = 0, and Hamilton's Equations will take on the form of 
the Equilibrium Problem : 

dQ r dP r n , 

~W = > ~di- = ' r = l,...,n. 

If we write their solution in the form : 

Q r = - P r , P r = Qf r , T = 1, , tt, 

we are led to the same solution of the original Hamiltonian 
Equations as before namely, that given by (7). 

3. Example. Simple Harmonic Motion. Here the kinetic en- 
orgy T and tho work function U are expressible respectively in 
the form : 

(1) T = ^q\ V -- \q*, 0<X. 
Thus 

(2) L = T+V-?-f 



(3) 



416 MECHANICS 

(4) ff-rt-L.-Lp. + lj.. 

Hamilton's Equations assume the form : 
al dq - p dp - - \ n 

a; di ~m' Tt~ A9 ' 

We propose to solve them by the method of 2. The equation 
for determining V, 2, (3), here becomes : 



We wish to find a function : 
(6) V 



which satisfies this equation.* One such function is enough. 
Let us see if we cannot find one in the form : 

(8) F = fl + W, 

where 12 = 12 (f) is a function of t alone, and W = W (q) is a func- 
tion of q alone. If this be possible, we shall have : 

' + V = o. 

This equation can be written in the form : 

X d!2 



The left-hand side of (9) depends on q alone, the right-hand side, 
on t alone. Hence each is a constant denote it by a ; it is 
obvious that a ^ : 

* Let the student disembarasa himself of any fears due to his ignorance of tho 
theory of partial differential equations. No such theory is needed in the kind of 
application in Physics which we are about to consider ; it would not even be help- 
ful in practice. The single function V(q, a) is obtained by a simple device fully 
explained in the text. 

There is, of course, a most intimate relation between the theory of Hamilton's 
Equations arid the theory of this partial differential equation, as is indicated, for 
example, by the " theory of characteristics" ; cf. Appendix C. The point is, that 
this theory is not employed in such applications as those illustrated here. For the 
latter purpose, a single solution V(q\, , q nt ai, , , is all that is required, 
and such a solution is obtained by ingenious devices of a homely kind, as set forth 
in this Chapter. 



SOLUTION OF HAMILTON'S EQUATIONS 417 

J_/dTF\ 2 + X 2==a 

The first equation gives : 

Q = a i f 

no constant of integration being added because we need only a 
particular integral, and so choose the simplest. From the second 
equation, 

(dW\ 2 
-j ) = 2ma m\q 2 . 

One solution of this equation is : 

W = I V2ma - m\q*dq. 

Thus 

/ 

(10) V=-o* + 

/ 



Equations (7), 2 here become : 



dq 

(11) __^_ ^_ 

fl_-^--<- m - Xg2 

u 

This last equation gives : 



and thus 

(12) q 

From the first Equation (11), 

(13) p = V2m^ cos \- ( - 0). 

Equations (12) and (13) constitute a solution of Hamilton's 
Equations, which, however, is at present restricted ; for we have 
not paid heed to Condition (7) on the one hand or, on the other, 



418 MECHANICS 

considered that the second equation (11) is restricted. Here 
then is a difficulty.* Either we must follow the theory as hitherto 
developed, using single-valued functions W and V ; then t is con- 
fined between certain fixed values. Or else we must introduce 
multiple-valued functions F, and then we must go back and 
revise and supplement the general theory. 

There is, however, a third choice a way out, whereby we 
can remain within the restrictions of the present theory. Accord- 
ing to that theory the solution given by (12), (13) is valid so long 
as 



Now, from the general theory of differential equations, Equa- 
tions a) admit a solution single-valued and analytic for the whole 
range of values oo<2<+oo. Equations (12), (13) yield 
a solution for a part of this interval. Therefore, by analytic 
continuation, the solution (12), (13) must hold for the whole 
interval. 

EXERCISES 

1. Obtain the solution of Equations a) in the form : 



(14) 

p = V2ma sin ^~ (t 

by choosing as W the function : 

W = I V2m<x m\q 2 dq + C(a), 

o 
and suitably determining the constant of integration C(a). 

2. Solve Equations a) directly, eliminating p and thus obtain- 
ing the equation 



* There is also a further difficulty, since the first equation (11) may not admit 
a solution (suppose p < 0), but this difficulty can be met by choosing the negative 



radical, 



V; 2ma 



SOLUTION OF HAMILTON'S EQUATIONS 419 
the general solution of which can be written in the form : 

-fi, ^ A. 

nit 

3. The Simple Pendulum. Let q be the angle of displacement 
from the downward vertical. Then 



m ml 2 . 9 Tr j 

T = - g 2 , U = mgl cos q ; 



Obtain the equation for motion near the point of stable equilib- 
rium: 



f 



dq 



where t is restricted. Hence discuss the two cases : a) oscil- 
latory motion (libration) ; b) quasi-periodic motion, when the 
pendulum describes continually complete circles (limitation). 

Observe that, when t passes beyond the restricted interval, 
the sign of the radical changes, and q changes from increasing to 
decreasing, or vice versa. 

4. Freely Falling Body, or vertical motion under gravity. 
Here, q shall be measured downward from the initial position. 



p = mq, 
p*- 



420 MECHANICS 

dW 
Since 



= V2ma + 2m 2 gq. 



_ dV dW 
P dq dq' 

we have no option as to which radical shall be taken. If the body 
is projected upward, q will bo negative for a while, and so we must 
choose the negative radical for this stage of the motion. At the 
turning point, (7) is not fulfilled, since d 2 V/dqda does not exist. 

We have now a new problem, as the body descends. The 
choice of W must be made on the basis of the positive radical. 
Nevertheless, both stages of the motion are covered by the solu- 
tion for the first stage : 

ft 1 2^y 

/> ft o\ 2 "%/_____ // ___ /9i 

p = mg (t /3) V2om. 
Why? 

4. H, Independent of /. Reduction to the Form, H' = Pi. 
We have seen in Chap. XIV, 5, Ex. 1, that if S be an arbitrary 
function of the q r , of n arbitrary constants, or parameters, the 
a r , and of t : 

where 

*'*' '"'*S ) * o, 



and if we set a r = P r , then the equations : 

fn\ dS ~ dS ., 

(2) p r = ^, Qr- W , r = l,...,n, 

define a contact transformation whereby Hamilton's Equations 
(4), 5, go over into (5), 5, and 

(3) H' = H + f t - 

If S does not depend on t, this equation reduces to the following : 

(4) H' = //. 

Suppose, furthermore, that H is also independent of t : 
H = H(q lf - - , q n , p lt - - , p n ). 



SOLUTION OF HAMILTON'S EQUATIONS 421 

Then 

H' = H'(Q l ,".,Q*,P l ,---,P n ). 

We propose the problem of determining S so that H r will depend 
only on the P r : 

H' = H'(P lt ,Pn\ 

and, in fact, that //' will be an arbitrarily preassigned function 
of the P r . Begin with the case : 

(5) H'(P 19 - , Pn) = P x . 

To find such a function S(q lt , q n , (x lt , a n ), consider 
the equation : 

, R v 

(6) 



Suppose it is possible to find a solution : 

W = W(q ly - , g n , A, 2 , ,) 

depending on n 1 arbitrary constants 2 , , a n and of 
course on h, which is also arbitrary such that* 

(7) 

(7) 



It then follows, as we will show later, that 

, 2 , , n 
This is the function which we will choose as S : 

(9) S(q l , - - , q n , a,, , a) = TT^, , tfn, A, 2, , ) 
where a t = A. If now we set : 

(10) Pj = ai = A ; P. = a., 5 = 2, , n, 
then (6) becomes, because of (2), (9), and (10) : 

(H) //(ft, , <?n, Pi, , Pn) = PI, 

and hence (4) gives : 

#' = PI, 

as was desired. 

* In practice this is done by writing down an explicit function of the nature 
desired, obtained by such artifices as the separation of variables. 



422 MECHANICS 

Thus the transformed Hamiltonian Equations become : 

dQ. 

-dt^ 1 ' 
(12) 



0, 



dt ' dt 
r = o, r = 1, ,n. 



2, 



The solution of this system is obviously : 

Ci = < + ft, Q> = P; s = 2, -,; 
P r = a r , r = 1, , n. 



(13) 



Returning, then, to the original transformation (2), which now 
takes on the form : 



{T dP r ' 



n, 



(14) p r = 

we liave : 



(15) 



The last n I of these equations can be solved for q 2 , , q n 
as functions of q 1 because of (7), thus determining the form of 
the curves of the natural path of the system. And then the 
first equation can be solved for q l in terms of t. This last state- 
ment is conveniently substantiated indirectly. All n equa- 
tions (15) can be solved for q l9 - - , q n in terms of t because of (8). 
These functions q r (t) satisfy the last n 1 equations (15), and 
so the earlier solution of these equations for q 2 , , q n in terms 
of q l become identities in t when q r is replaced by q r (t) given by 
using all n equations. 

Proof of Relation (8). Observe that Relation (6) is an identity 
in the h, a a as well as in the q r . Hence on differentiating suc- 
cessively with respect to h, a 2 , , a n , we find : 



+W^ + 



(16) 



+ + 



SOLUTION OF HAMILTON'S EQUATIONS 423 

The determinant of these equations is the Jacobian that appears 
in (8). If it were 0, it would be possible to determine n multi- 
pliers \i, , X n , not all 0, such that the n equations : 



(17) 



= 



= 



are true, and since (7) holds by hypothesis, \ may be chosen at 
pleasure. Now multiply the fc-th equation (16) by X* and add. 
The coefficient of each H p vanishes, and so the whole left-hand 
side reduces to 0. But the right-hand side is X u which is arbi- 
trary. This contradiction arises from supposing that (8) is not 
true, and the proof is complete. 

The Equation of Energy. When the kinetic energy T and the 
work function U are both independent of t, H is also independent 
of t, and H represents the total energy (sum of the kinetic energy T 
and the potential energy U). Hence* // is constant and we 
may write : 

h = H(q i9 - - , q n , p l9 , p). 



Thus this equation appears to be derived from the physics of 
the problem. It is. But this derivation is not helpful in the 
present theory. For we are dealing with contact transforma- 
tions which reduce Hamilton's equations to a desired form, and 
Equation (6) takes its systematic place in that theory. It ex- 
presses a condition for the function W that will make the desired 
transformation possible. Nevertheless, the physics of the situ- 
ation throws a side light on the situation, which it is well to note. 
The Symmetric Form. We have set, unsymmetrically, h = P l 
in Equations (10). We might equally well replace (10) by the 
equations : 

(100 *(Pi, , Pn) = A, P* = ., = 2, , n, 



where <i> (a lt , a n ) is any function such that cfa/d^ 5^ 0. The 
above reasoning, with an obvious modification in detail, shows 
that the determinant : 

*That H is here constant along a natural path follows from Chap. XI, 3 : 

dH dH 

Tt - IT - ' 



424 MECHANICS 

d(W q , - - , W Q ) 

(8') ~^ -^ * 0, 

3(a lf <* 2 , , a) 

where W = W(q ly , q* 9 h, a lt , n ) is determined as before 
from (6), and h = $(!, 2 , - , ). Thus the transforma- 
tion (14) is justified and Equations (12) become : 



(120 



dQ r 

dt 



- 

dt 



1, , n. 



The solution of these equations is obvious, and symmetric. 
First, 

P r = a rt r = 1, , n, 

where the a r are n arbitrary constants. Next, 

Qr = U r t + Pr, r = 1, , H, 

where 

o> r = $r(<*i, , a n ), r = 1, - , n, 

and the f} r are n arbitrary constants. Thus we have, finally : 

(19) , . 

ft, 

a wholly symmetric solution of Hamilton's Equations. 

If we should wish to use a function $(0^, , a n ), for which 
some other derivative, as d$/da z , is ^ 0, then we should need 
a solution W(q lt , q n , a lt - , a n ) such that 



5. Examples. Projectile in vacuo. Let a particle of mass 
m be acted on solely by gravity, and let it be launched so that it 
will rise for a time. Let q lt q 2 , </ 3 be its Cartesian coordinates, 
with q l vertical and positive downward. Then 

T = & 2 + ft 2 + </s 2 ), I/ 



SOLUTION OF HAMILTON'S EQUATIONS 425 

tt = ^ Cpl2 + p * + P ^ 
The equation for W becomes : 



Let us try to find the desired function, 



0(a, f a,) ' 

by setting 

W. = W, + W 2 + W 3 , 

where W r = W r (q r ) is a function of q r only. Thus 



n 
0. 



"j i j 

Vd^/ Vrf? 2 / Vrf 

Since it is only a particular function W that is needed, satisfy- 
ing the Jacobian Relation of Inequality, 4, (8), it will suffice 
to set 



^J 2 = 2m(/l-a 2 2 -a 3 2 )- 

Herc, h is determined by the initial conditions from the equation 
H = A, and 2 > <*3 are anv ^ wo parameters such that initially 

2m (h c* 2 2 3 2 ) + 2m 2 gq l > 0. 
We now may choose : 

JTTf 

* -v/O TTZ A /O O Q 

where 8 is positive, negative, or zero, subject merely to the rela- 
tion of inequality. But, in the choice of W lf it is the negative root, 



- a,* - a,*) 
that must be chosen, since 



_ _ dW l 
Pl J 



426 MECHANICS 

and p 1 < in the stage we are considering. We may take 

0i 
W 1 = - CV2m(h - 2 2 - a 3 2 ) + 2m 

Cl 

where c x is the initial value of q r Thus, finally, 

Q\ 

W = - A/2m(A - <* 2 2 ~ 3 

c, 

The condition (7), 4, is satisfied. 

We are now in a position to write down the solution of the 
problem. It is given by Equations (15), 4 : 

t + ff =^=- m f _ ^i 

dh J V2m(h - 2 2 - 3 2 ) + 2m*gq l ' 

A = |^ = 2ma a f 
8. J 



along with the equations : 



The first of the equations in each of these sets of three is in 
substance identical with the one which governs the vertical 
motion of a falling body, 3, Exercise 4, where now 

a = h - <* 2 2 - 3 2 , ]8 = - ft ; 
and hence : 



- 



- 2 2 - 3 2 ) 

In the earlier case, (7 = initially, and so c t mnst be set = 0. 
The last two equations in the first set give : 

ft) 



SOLUTION OF HAMILTON'S EQUATIONS 427 
and so, finally : 



s = 2, 3. 



The method we have employed gives the solution of the prob- 
lem so long as the body is rising no longer ; for when it is 
descending, p v becomes positive, and dW l /dq 1 = dW/dqt cannot 
be expressed by the negative radical. This second stage of the 
motion, in which the body is falling, could be dealt with by apply- 
ing the method afresh with suitable modifications in particular, 
by taking the positive radical for dW t /dq^ But this step can 
be eliminated if we observe that the equations we are integrating, 
Hamilton's Equations, here become : 



di ~m Pr > 



dt 



r = 1,2,3; 



di 



2,3. 



The solution of these equations is unique, and is expressed by 
functions of t which are analytic for all values of L Hence the 
analytic continuation of the restricted solution found above gives 
the general solution, and the formulas found for q r , p r are true 
generally. 

EXERCISES 

1. Central Force, two dimensions, attracting according to the 
law of nature. Let q l = r, q 2 = <p. Then : 



= R 



2m\dr 



428 MECHANICS 

/dR\* n , . 2wX a 2 
(W) =2mA + -^ 

Thus 



W= 2mh + -^dr + <*>, 

J T T 

r* 

where either the plus sign or the minus sign holds throughout 
the first stage. Hence 

r 

dr 



t + 



= + m f 
~ J 



Vo z, , 2mX 
2mh H 
r 



02 = 



2mh 



r r 

Discuss the case that the radicand vanishes for two distinct 
positive values of r, expressing r as a periodic function of ^>, and 
evaluate the integral that expresses t ; cf. 9. 

2. The same problem in space. Let q l = r, q% = 0, q z = <p ; 
x r cos 6 cos ^?, 2/ = r cos 6 sin ^?, 2 = r sin ; 



~2m 

TT = fl + + *; 
2m\ 



J VO 



Complete the solution and discuss the cases that the radicands 
have distinct roots. 



SOLUTION OF HAMILTON'S EQUATIONS 429 

3. Discuss the problem of 4 when n = 1. Show that W is 
given by solving the equation : 



and integrating : 

= ef " ^ dh 

I 
W 

Then 



ff(q,h)dq. 



_8W 
y dP 

Thus 



"- 8q- 

6. Comparison of the Two Methods. We have studied two 
methods of solving Hamilton's Equations, a) Reduction to the 
Equilibrium Problem ; b), when // does not depend on t, Reduc- 
tion to the Form, //' = P v 

The first method, being general, must apply to the second case. 
It does. Let us treat this case by the first method, as set forth 
in the Exercise of 2. We will choose as V the function : 

(1) V = - ht + W, 

where W = W(q lt , q n , h, a a > * > n) is the function of 4, 
and h, a s have been replaced by P lt P 8 . The transformation of 
that Exercise, 

r)V ?)V 

(2) p r = ~ Qr r = 1 n 

yields an H ' that vanishes identically. The transformed Hamil- 
tonian Equations thus take the form : 

(Ti ^ r n ^ r n r 1 . . . n 

W -dT-' dt ~' r ~ lj ' n * 



430 MECHANICS 

Departing from the notation of the Exercise, write their integrals 
in the form : 

... I Qr = Pr, r = !,--,; 

(4) 1 

I P, = h, P. = a., s = 2, ,n. 

The solution of the original Hamiltonian Equations is now given 
by substituting these values in (2) : 



= 8V 

(5) 



* = 2, . . , n. 



But 

3V_ = 3W W = _ 3W 3V = 
^ * dq r ~ dq r ' dh + dh ' da, ~ da,' 

Hence Equations (5) agree not only in substance, but even in 
form, save for one exception, with Equations (15), 4. The 
equation arising from differentiation with respect to h in the 
earlier case read : 



Here it is : 



7. Cyclic Coordinates. It frequently happens that H, besides 
being independent of t, contains fewer than n g's. Begin with 
the case of one q, 

(1) H = H(q l9 p lt ---,p n ). 
From Hamilton's Equations, 

(2) f-f-0. -.-., 

and hence 

(3) ?> = , 5 = 2, , n. 

It is not difficult to complete the solution by means of Hamil- 
ton's Equations and the integral of energy, 

(4) h = H(q l9 p 19 ,p n ); 



SOLUTION OF HAMILTON'S EQUATIONS 431 

but this is not the form of solution in which we are interested. 
We desire a discussion by the methods of 4 ; in particular, by 
the transformation : 

dW 



/*\ 
(5) 

where 

(6) W = W( qi1 - , ?, h, a - , a n ) 

is a solution of the equation : 



m \ 

l , ,..., J, 



,,,..., 

- 



and P l = A, P, = a a , s = 2, , n. 

To find such a solution we turn to the Method of Separation 
of Variables, which has rendered such good service in the past. 
Let 

'(9) . w=W l + -- + W n , 

where W r = W r (<?r) is a function of q r alone and of the n 
parameters, A, a 2 , , . From (5) and (3) we see that 



a " 2, - - - , n, 

and so we try : 

TT, = g., s = 2, - - , n. 

Let T^! be denoted more simply by v : 

(10) W, = ^(fc^afc-'-.aO =t>. 
Then (7) becomes : 

(11) fl r (g 1 ,^,a 2 ,---,n)=A. 

If we assume that 

fiff 
(12) l^ffp.feuPi."*'--.*..)* ' 

^Pl 

and solve the equation : 
(13) 



432 MECHANICS 

for p, : 

(14) p, =*(? A, 2 , ',), 
we have : 

(15) -^ = *(?i, A, a,, -,). 

Now choose as : 

i 

(16) v = J *(<?i> A, a 2 , , a.) dq lt 

C 

where c is a numerical constant. 
We are thus led to a function 

(17) W = V + otf, + + a n q n 

of the desired kind, provided the Jacobian relation (8) is satisfied, 
The Jacobian here reduces to 



d' 2 v 



" ' r ' 



dq.dh " dh' dh' 

where p 1 is determined by (13). On differentiating (13) -we find : 

M!! 

dp, dh 

and so the Jacobian does not vanish. 

Solution of Hamilton's Equations. We can now apply the 
general theory of 4. The transformation (5) of the present 
paragraph carries Hamilton's Equations over into the form: 



= 0, r-l,-..,n, 

the solution of which is : 

ft = + fc, Q. = A, s = 2, ..-,n; 
P x = A, P, = a a , s = 2, - - - , n. 

These values for Q r , P r are to be substituted in (5), and the result- 
inc eauations solved for q r , p r : 



SOLUTION OF HAMILTON'S EQUATIONS 433 

<7i 

dh J dh l9 



aw 

dh 



8W r , , . 

Pi = - = *Wi, h, a 2 , , a n ), 



(18) 



dW 

p 9 = -7T-- = a,, s = 2, , n. 

The equations of the second line determine g. as a function 
of ft: 

/' (W 
~^~dq ly s = 2, '--,n. 

8 

The first equation gives ft as a function of t. 

EXERCISE 

Obtain the final result (18) directly from Hamilton's Equations. 

8. Continuation. The General Case. Let H depend on 
1 < v < n arguments qk : 

(1) H = #(ft, -,??!, ,pn). 

The method of treatment is similar, though the solution cannot 
in general be obtained by quadratures. Equations (3) of 7 
now become : 

(2) p, = a., s = v + I, , n. 

By analogy we now seek to determine W in the form : 

(3) W = v + a* +l q r+1 + + a n q n , 

(4) v = *(? ,<?, h, 2 , , ), 



(5) 

a^T 



434 MECHANICS 

Equation (7), 7, for W now becomes : 



/ c \ L rj 

(b) n = //^ft, - , q,, TT-, , Tjjp a^+i, , 

This is an equation of the same type as (6), 4, but with v < n 
variables q r . As in the earlier case, only a particular solution 
is sought, and such a solution may be found by special devices, 
notably the method of separation of variables. 
A function v once found, the solution proceeds as before. 



(7) 



/Si = - + qi, I = v + 1, , n. 



From the equations of the second line g* can be found in 
terms of ft, k = 2, - , p. From the first equation ft is now 
found in terms of t. Finally, qi is given by the last line, 

I = v + 1, , n. 

9. Examples. The Two-Body Problem. Consider the motion 
of two bodies (particles) that attract each other according to 
the law of nature and are acted on by no other forces. Their 
centre of gravity travels in a right line with constant velocity, 
or else remains permanently at rest. We will assume the latter 
case. Then each of the bodies moves as if attracted by a force 
at 0, the centre of gravity, which is inversely proportional to 
the square of the distance of the body from 0. 

We will first discuss the motion in a plane later, in space. 

Let the particle be referred to polar coordinates, ft = r, 
g 2 = (p. Then 



" 2\dt 2 dt 2 
Hence 



Let 

W = v + a 2 q 2 . 



SOLUTION OF HAMILTON'S EQUATIONS 435 
Then v is given by the equation : 

1 f/^\ 2 , 2 2 1 ^ _ 
2m \\dq l / (7j 2 J q l ' 
or 



rt 7 . 2mX <* 2 2 , 

2mA H 1- dr. 

r r 2 ' 



where a definite one of the two signs holds for the first stage of 
the motion. 

Equations (18) of 7 now give the solution of Hamilton's 
Equations in the form : 

. ^ dv /* Sv . 



or 



,=/- 

c 



dr 



2mh + 



2m\ 



ft = 



The directness of the result is particularly noteworthy. It 
has not been necessary to make use of skillful devices or to effect 
complicated eliminations. From the evaluation of the second 
integral r can be expressed as a trigonometric function of <p. But 
the discussion of r in terms of t is more complicated ; cf . below 
the reference to Charlier. 

The Orbit in Space. To treat the motion in three dimensions 
let 

x = r cos cos <p t y = r cos sin ^>, z = r sin 0. 

Then 



Let 



0, 



Then 



Pi 



Ps 



436 MECHANICS 

H = ( v * + Si P 2 



2m \ I tf, 2 ?, 2 cos 2 ? 2 / q l 
Since H = H(q v q^, p 1( p a , p 3 ), we see that p 3 = a 3 (const.)- Thus 

W = v + ci^s, 
where v is given by the equation : 

J_[7-^Y + A. fi?Y 4. * 2 i _ x = , 

2m lA^/ qf\dqj q, 2 cos 2 q. 2 J q l 

Hero, t-hcro arc only two independent variables, q^ = r and 
g. 2 = 6. The equation can be written in the form : 



0. 

cos 



On setting 

v = R + 

the variables can be separated : 

- r*(~^ + 2mhr* + 2m\r = 
Hence 



ft 



y 



ft 

= rv^ _ a ., 2 



where the signs are determined for a particular stage of the motion, 
and c, T are arbitrary numerical constants. Adding the further 
term a 3 g 3 , we have: 

W = v + ag^, v = R + 0. 



We are thus led to the solution of the problem in the form given 
by (7), 8: 



SOLUTION OF HAMILTON'S EQUATIONS 

, +A -.A * 



437 



(2) 



&=- 



r 

dr 



J . 9^/0 T, 2raX a, 2 

c r 2 \2rnh -\ \ 

* r r 2 

6 

d6 



- a 3 2 sec 2 



v a, 2 2 a 3 2 sec 2 



The discussion of this solution on the hand of the explicit 
evaluation of the integrals and the inverse functions thus arising 
presents practical difficulties. The problem is of so great impor- 
tance in Astronomy that it has been treated at length by Charlier, 
Mcchanik des Himmels, Vol. I, Chap. 4, p. 167. On p. 171, 
Equations (7) are identical with our solution, save as to notation. 

Failure of the Method. There are cases in which the method 
breaks down. Consider, for example, motion in a plane. Sup- 
pose the body is projected from a point A, distant a from the 
centre of force, 0, at right angles to the line OA and with a velocity 
v (} such that 



It will then describe a circle, r = a. But the Equations (1) 
or (2) can obviously never yield this solution. Why? 
The function v was determined from the equation : 



= 2mA 



2raX 



In the present case, 



h =- 



2a' 



mav , 



and hence 



= 0. 



438 MECHANICS 

Thus the condition 



is not fulfilled, and so, of course, there is no reason why the method 
should apply, since the hypotheses on which it depends do not 
hold. 

10. Continuation. The Top. We take over from Chapter 
VI, 18, the expression for the kinetic energy, 



By Euler's Geometrical Equations, this becomes : 
T = 



Let 

tfl ^ Q> <?2 = <P> 

Then, since 

= dT 

we have : 

Pi = Ad, 



p s = C<p cos + ( A sin 2 + C cos 2 
Thus T, expressed in terms of the p's and <?'s, becomes : 



Furthermore,* 

U = Mgb cos 0. 
Thus 



Hence it appears that the problem comes under the case of 
cyclic coordinates treated in 7. First, then, 



* It is necessary to change from the earlier notation h for the distance from 
the peg to the centre of gravity, since h plays so important a rdle in the present 
theory. Let the distance be denoted by 6. 



SOLUTION OF HAMILTON'S EQUATIONS 439 
To determine v we have : 

Irl dv* , 1 9 . l/a 2 cosq 1 - a 3 \ 2 1 . ,_ , L 

2 Li 55? + C^ + l( sin gl ) J + M * 6 COS * - * 

^2 

sin 2 ft ^2 = (24 A - La 2 2 - N cos ft) sin 2 q l - ( 2 cos q 1 - 3 ) 2 , 



_ 
= r+ V(2^ A - La 2 2 - JV cos ft) sin 2 g, - ( 2 cos ?, - ^ 
t/ sin ft ?1> 

c 

where is an arbitrary numerical constant, not a parameter, 
and the sign of the radical must be chosen with respect to the 
special stage of the motion under consideration. Moreover, for 
brevity, 

L = 4, N = 2AMgb. 

v/ 

The solution of the problem, as given in 7, now takes on the 
form: 

+*-* 



Thus 

A sin ft ( 



4- C- 

'~e/~H 



v (2Ah L 2 2 ~ A^ cos gj sin 2 gj ( 2 cos gj a s ) 2 

Let 

u = cos #,. 

Then this equation becomes : 



9l = r ^ 

c 



cose, 

e/ +V/<W 

where 



This is the same result obtained by elementary methods, 
Chap. VI, 18. But compare the technique. With only Euler's 



440 MECHANICS 

Dynamical and Geometrical Equations to work with,* elimina- 
tions had to be made by ingenious devices, whereas the present 
advanced methods free the treatment from all artifice. The 
fundamental equation in desired form is evolved naturally, directly, 
from the general theory, not untangled from a snarl of equations. 
Instead of having to solve three equations for 6, <j>, \j/ by more or 
less ingenious methods of elimination, the functions 7 7 , [7, and 
hence H are obtained without the use of any artifice whatever, 
and the method of 7 yields q l at once as a function of t, the 
further equations giving q 3 = <p and </ 3 = \f/ immediately. 

EXERCISE 

Study the motion of a top with hemispherical peg, spinning 
and sliding on a smooth table. Show that 



where 

F(u) = (2h - ^ - 

11. Perturbations. Variation of Constants. In the problem 
of perturbations the motion which the system would execute if 
only the major forces acted is regarded as fundamental, and 
then the variation from this motion due to the disturbing forces, 
thought of as slight, is studied. 

This analysis of the physical problem is mirrored mathematically 
by writing down Hamilton's Equations for the actual motion : 



___ -.- 

~dt ~Wr dt" dq r ' ' '' 

and then setting the characteristic function H of the actual prob- 
lem equal to the H of the problem due to the major forces, plus 
a remainder, H l : 

(2) H = H, + H { . 

* It is true that in the earlier treatment we had two integrals of the differen- 
tial equations of motion to work with at the outset, namely ; the equation of energy, 
T = U + h, and the equation arising from the fact that the vector moment of mo- 
mentum <r is always horizontal. But even so there were three equations in 0, $, <f> 
to integrate. 



SOLUTION OF HAMILTON'S EQUATIONS 441 

Transformation of the Major Problem to the Equilibrium Problem. 
First, the major problem, represented by Hamilton's Equations 
in the form : 



is solved by reducing it, through a contact transformation, to 
the Equilibrium Problem. The contact transformation is given 
by the equations : 

fA\ 

(4) Pr r 
where 

(5) F = F(<7i, , q, P,, , Pn, t) 

is obtained as follows. Write down Jacobi's Equation, cor- 
responding to Hamilton's Equations (3) : 



Let 

V = Vfe, -,?, a lf ", a n , 

be a solution of this equation such that the Jacobian 



O / v 7~ VJ. 

0(a l9 - , a n ) 

In this function, replace a r by P r . The resulting function is the 
function (5). [In practise, the function F ^, - , q ny a lf , 
a n , t) is obtained, not from an elaborate theory of partial differ- 
ential equations, but by means of simple devices, ad hoc.] 
Let the transformation (4) be written in the explicit form : 



,. f Qr = Fr(p lt ' * ' 9 Pn 9 qi, ' * * 9 qn, 

I P r = G r (p lt ' jpniQi, ' " ,qn, 

or 

f 9r = fr(P , P, Q -^Qn, 

1 p r = g r (P ly ' , P n , Q 19 - , On, 



To say that the major problem is thereby transformed to the 
Equilibrium Problem means that, when the variables q ry p r that 



442 MECHANICS 

form the solution of Equations (3) are subjected to the transfor- 
mation (4), the resulting Hamiltonian Equations become : 

(7) f = 0, ^ = 0, r=l,..-,n. 

The solution of these equations can be written in the form : 

(8) Q r = 0r, Pr = r, f = 1, , ft, 

where a r , Pr are constants. Now transform the variables Q r , P r 
that are the solution of Equations (7), namely, the functions 
given by (8), back by means of the transformation (4"), and we 
have the solution of Equations (3) in the form : 

f Qr = /r(i, ' ' ' , n, ft, , 0n, 
1 Pr = 0r(a lf " -,, ft, ' ',0, 

Thus the transformations (4 ; ) or (4"), and (9), identical 
except in notation, represent two distinct things: 

a) In the form (4") these equations represent the Contact 
Transformation (4). 

b) In the form (9) they represent the Solution of the Hamil- 
tonian Equations of the Major Problem, or (3). 

Transformation of the Actual Problem by the Same Contact Trans- 
formation. We now proceed to apply the contact transformation 
(4), not to the variables (q r , p r ) which satisfy Equations (3), 
but to the variables (q r , p r ) of the original problem, which satisfy 
Equations (1). Since this is a contact transformation, we know 
that Equations (1) will go over into new equations of the same 
form: 

dQ,_8ir dPr__9ff' j. 

(W) dt ~ dP r ' dt ~ Wr ' ' 

Here H' = H'(Q r , P r , <) has the value, cf. Chap. XIV, 5, Ex. 1, 
(15): 

(11) H' = H + 

But from (6) : 



Hence 

H' = H - 



SOLUTION OF HAMILTON'S EQUATIONS 443 

Finally, from (2) it follows that 

(12) H f = ff t . 

Thus Equations (10) take the form : 

dQr^dH, dP r _ m, 



The result may be stated as follows. When the variables q rj p r 
which form the solution of the actual problem represented by Equa- 
tions (1) are transformed by the contact transformation (4) or (4'), 
the transformed equations take the form (13), where H l is the given, 
or known, function of Equation (2), now expressed through (4) or 
(4") in terms of Q r , P r , t. 

The Final Solution. It is now but a step to the solution of 
Equations (1), which represent the actual problem. Solve Equa- 
tions (13), thus determining Q r , P r as functions of t. Then 
transform these functions, the solution of (13), back by means 
of (4) or (4") to the variables q r , p r . The latter satisfy Equa- 
tions (1). 

The result can be expressed in the form : 



(14) 

Pr =flTr(P,, ,Pn,Qi, ' ' ' , Qn, 

where Q r , P r arc determined by Equations (13). 

Variation of Constants. The method above set forth has been 
called the "variation of constants." This expression is a mathe- 
matical pun. It is a pun on the letters a r , r . These, in Equa- 
tions (9), are constants the equations there representing the solu- 
tion of the major problem, (3). On the other hand, they can be 
identified with the variables P r , Qr of (14), these variables being 
determined by (13), and then Equations (14) represent the solu- 
tion of the actual problem, (1). 

We can attain complete confusion of ideas, as is done in the 
literature, by changing the notation in (13) and (14) from 
Q r , P r to r , oL r . Thus (14) goes over into the form of (9), and 
(13) is replaced by the equations : 

da r _ 3(- g,) df)r _ B(- H,) 

dt ~ d0 r ' dt ~ da r ' r - L >'"' n > 



444 MECHANICS 

where H 1 = H 1 (Q r , P rj t) is now written as H l (ft 1) a 1) t) ) the 
Hamiltonian function now being H 1 instead of ff,. 

Thus the pun is explained but it is a poor pun that has to be 
explained. 

12. Continuation. A Second Method. It is possible to treat 
the problem of perturbations in still another manner. Let 
<f>(a lf , a n ) be any given function whose first partial deriva- 
tives are not all 0. Let the Hamiltonian Equations for the undis- 
turbed motion, namely, (3), be transformed by a new contact 
transformation : 



where S is defined as follows. Consider the equation : 



/i/r\ / \ T 

(16) *(,, -..,.) = 

Let 

, q n , !,--, a n , t) 



be a solution such that * 



Now, make the contact transformation : 

/1>7\ ^ r> ^ 

(17) Pr - Wr , Pr=~ W , 

where 

5 = 8(q ll , q^ Q,, , Qn, 0- 

* In order to find such a solution, begin with the equation : 

, / OS dS \ , dS 

h =H( qi ,..., qn ,~,...,--,t) + -, 

where h is an arbitrary constant, and seek a solution : 

S = S (<?,, , q n , h, 2 , , On, Of 
such that 



t g t , ' ' ', Qn 

d (h, as, -, ) 
where as, , On are arbitrary. Substitute 

h = <p (ai, , a n ) 
in iS. If d<p/dai ^ 0, this will be the function desired. 



SOLUTION OF HAMILTON'S EQUATIONS 445 

This transformation, applied to Equations (1), carries these over 
into equations of the same type : 

dt dP r ' dt 8Q r ' ' ' ' 

where, by Chap. XIV, 5 : 

(19) H' = H + ?j- 

VI 

But, by (16) and (17) : 
Hence, with the aid of (2) : 



the arguments now being the Q ry P r into which g r , p r have been 
transformed by (17). Thus Equations (18) take the form : 

dQr = 0/7, dP r _ _ 3/7, _ 3jp 

" r - 1 "' n - 



Solve these equations and substitute the functions of t thus 
obtained, namely, the Q r , P r , in (17). The functions q r , p r of t 
obtained from these equations are the solution of the actual prob- 
lem, or Equations (1). 

Carathgodory * treats Equations (20) as follows. He writes 
X//! instead of H 1 : 



He then develops the solution into a power series in X : 

f Qr = Ct r + \Cl r + X 2 C 2r + , 
< 22 > ( P r = r -v a t+ Wlr + ' ' , 

where C*r, D kr are functions of t, vanishing when t = (for sim- 
plicity we have set t = 0). On substituting these values for 
Q r , P r in (21) and equating coefficients of like powers of X, the 
coefficients C* n Dk r can then be obtained by quadratures. 

* Cf. reference above, p. 381. The page in R.-W. is 211. 



APPENDIX A 
VECTOR ANALYSIS 

In Rational Mechanics only a slight knowledge of Vector 
Analysis is needed. It is important that this knowledge be 
based on a postulational treatment of vectors. The system of 
vectors is a set of elements, forming a logical class. Certain 
functions of these elements are defined, whereby two elements 
are transformed into a third element. These functions are called 
addition, multiplication by a real number (here, only one element 
enters as the independent variable), the inner product (scalar 
multiplication), and the outer product (vector multiplication). 
The functions obey certain functional, or formal, laws, which 
happen to be a subset of the formal laws of algebra : 

A + B = B + A 



AB = BA 

A(BC) = (AB)C 
A (B + C) = AB + AC 
(B + C)A = BA + CA 

A brief, systematic treatment such as is here required is given 
in the Author's Advanced Cakulus, Chap. XIII. For a first 
approach to the subject the Hamiltonian notation of S and V for 
the scalar and vector products has the great advantage of clear- 
ness in emphasizing the functional idea the concept : transfor- 
mation. On the other hand the notation pretty generally adopted 
at the present day is the designation of vectors by Clarendon or 
boldface, the scalar product being written as a b or ab (read : 
a dot b), and the vector product as a X b (read : a cross b). It 
is useful, therefore, to have a syllabus of definitions and essential 
formulas in this notation. 

447 




448 APPENDIX A 

1. Vectors and Their Addition. By a vector is meant a directed 
line segment, situated anywhere in space. Vectors will usually 
be denoted by boldface letters a, A, or by parentheses; thus 
a vector angular velocity may be written (w). 

Two vectors, A and B, are defined as equal if they are parallel 
and have the same sense, and moreover are of equal length : 

A = B. 

By the absolute value of a vector A is meant its length ; it is 
denoted by | A |, or by A. 

Addition. By the sum of two vectors, A and B, is meant their 
geometric sum, or the vector C obtained by the parallelogram 

law: 

A + B = C. 

In order that this definition 
may apply in all cases, it is 
necessary to enlarge the system 

of vectors above defined by a nul vector, represented by the 

symbol 0. 

If B is parallel to A and of the same length, 

but opposite in sense, then 

A + B = 0, or B = - A. B 

FIG. 149 

Moreover, we understand by wA, where m is 
any real number, a vector parallel to A and m times as long ; its 
sense being the same as that of A, or opposite, according as m 
is positive or negative. If m = 0, then raA is a nul vector : 
OA = 0. The notation Am means wA, and also 

aA + 6B a . , 6 _ 

r- j means . , A H rr B. 

a + o a + o a + o 

Vector addition obeys the commutative and the associative law 
of ordinary algebra : 

A + B = B + A 

A + (B + C) = (A + B) + C 

Subtraction. By A B is meant that vector, X, which added 
to B will give A : 

B + X = A, X = A - B. 




VECTOR ANALYSIS 449 

To obtain X geometrically, construct A and B with the same 
initial point ; then A B is the vector whose initial point is the 
terminal point of B, and whose terminal point is the terminal 
point of A ; Fig. 149. 

Cartesian Representation of a Vector. Let a system of Cartesian 
axes be chosen, and let i, j, k be three unit vectors lying along 
these axes. Let A be an arbitrary vector, whose components 
along the axes are A lt A 2J A z . Then evidently 

A = AJ + A 2 j + A z k. 

E = B,i + B,j + B,k t 

then 

A + B = (A, + BJi + (A, + B,)j + (A, + 3 )k. 
Also : _ 

A ^ 



Resultant. If n forces, F x , F 2 , , F n , act at a point, their 
resultant, F, is equal to their vector sum : 

F = F t + F 2 + + F n . 

If n couples, M u M 2 , , M n , act on a body, the resultant 
couple, M, is equal to their vector sum : 

M = MJ + M 2 + - + M n . 

Two or more vectors are said to be collinear if there is a line 
in space to which they are all parallel. In particular, a nul vector 
is said to be collinear with any vector. Three or more vectors 
arc said to be complanar if there is a plane in space to which they 
are all parallel. In particular, a nul vector is said to be parallel 
to any plane. If three vectors, A, B, and C, are non-complanar, 
then no one of them can vanish (i.e. be a nul vector) and any 
vector, X, can be expressed in the form : 

X = ZA + mB + nC, 

where Z, m, n are uniquely determined. 

Differentiation. Velocity. Acceleration. Osculating Plane. A 
variable vector can be expressed in the form : 

A = 



450 APPENDIX A 

where i, j, k are three fixed vectors mutually perpendicular. If 
/(Oi <p(t), ^(0 have derivatives, the vector A will have a de- 
rivative defined as 



lim-rr = 



Its value is : 
Moreover, 



If m is a function of x and A is a vector depending on x> and if 
each has a derivative, then mA will have a derivative, and 

d(mA) dm. . of A 

-~^j - = -y~ A + m ~T' 
ax ax ax 

If a point P move in any manner in space, its coordinates being 
given by the equations : 



where /, <p, $ are continuous functions of the time, having con- 
tinuous derivatives, and if 

r = xi + yj + zk, 
the vector velocity of P is represented by 



W /i <f>, t have continuous second derivatives, the vector 
acceleration of P is given by 



The plane determined by the vectors r and f drawn from P 
(on the assumption that neither is a nul vector) is the osculating 
plane. Thus the vector acceleration always lies in the osculating 
plane. 

2. The Scalar or Inner Product. The scalar or inner product 
of two vectors, A and B, is defined as the product of their absolute 
values by the cosine of the angle between them. It is denoted 
by A-B or AB and is read: "AdotB." Thus 

A - B = AB = | A | | B | cos c. 



VECTOR ANALYSIS 451 

If one of the factors is a nul vector, the scalar product is defined 
asO. 
The commutative and the distributive laws hold : 

AB = BA 

A(B + C) = AB + AC. 

The associative law has no meaning. 

The scalar product vanishes when either factor is a nul vector ; 
otherwise when and only when the vectors are perpendicular to 
each other. Furthermore : 



often called the norm of the vector. 

:2 i ;2 i k2 _ i 

ii, j i, K i, 

jk = 0, ki = 0, ij = 0. 
Cartesian Form of the Scalar Product : 

= AB 
Differentiation : 

If a is a unit vector, i.e. if | a | = 1, then 

a 2 = 1, and aa' = 0. 

3. The Vector or Outer Product. Let two vectors, A and B, 
be drawn from the same initial point. Then they determine 
a plane, M, and a parallelogram in that plane. The vector 
or outer product is defined as a vector perpendicular to M and 
of length equal to the area of the parallelogram. Its sense 
is arbitrary. It is defined with ref- AXB 
erence to the particular system of 
Cartesian axes to be used later. It is 
denoted by 

AXB 

and is read : " A cross B." FIG. 150 




452 



APPENDIX A 



If one of these vectors is 0, or if the vectors are collinear, neither 
being 0, the vector product is defined as 0, and these are the 
only cases in which it is 0. Otherwise, let e be the angle between 
the vectors. Then 

| A X B | = | A | | B | sin c. 
The commutative law does not hold in general, for 

AXB=-BXA. 

The associative law does not hold ; e.g. (i X j) X j 5^ i X (j X j). 
But the distributive law is true : 



and 



C)=AXB 



as c^n be proved geometrically, or still more simply, analytically, 
by means of the Cartesian form ; cf . infra. 

It is convenient to choose the sense of the vector product so 
that 

i X j = k, j X k = i, k X i = j. 
In any case 

A X A = 0, 
and so, in particular, 

i X i = 0, j X j = 0, k X k = 0. 

Cartesian Form of the Vector Product : 

A X B = 



i J 

**l -^- 



Differentiation: 



- 

dx 



dx 



- 

dx 



4. General Properties. Let A, B, C be three non-complanar 
vectors drawn from the same point. The volume of the paral- 
lelepiped determined by these vectors is numerically 

A (B X C). 



VECTOR ANALYSIS 



453 



A necessary and sufficient condition that three vectors A, B, 
C be complanar is : 

A - (B X C) = 0. 

Linear Velocity in Terms of Angular Velocity. Let space be 
rotating about an axis / with vector angular velocity (w). Then 
the velocity v of an arbitrary 
point P will be : 




v = () X r, 

where r is the vector drawn 
from any point O of the axis to 
the point P. If the axis passes through the origin, then 



Fia. 151 



v = 



J 



x y 



and 



v x = zwy yw z 

Vy = Xtl)g Z<l) X 



If it passes through the point (a, 6, c), then 

v x = (z - c) co y - (y - 6) w z 

v z (y 6) o) x (x a) u y 

In tho general case of motion of a rigid body (i.e. motion of 
rigid space), lot 0' : (z , y , z ) be a point fixed in the body, and 
let (f, ??, f ) be the coordinates of any point P fixed in the body, 
the origin being at 0' ; but otherwise the (, rj, f )-axes may 
M p move in any manner. Then 




FIG. 152 



O' 



where 

P 7 

COf CO, C0 

* i r 



V = V + V', 



v = 



454 APPENDIX A 

Localized Vectors. It is sometimes convenient to prescribe the 
initial point of a vector, or the line in which the vector shall lie, 
as in the case of a force acting on a particle, or a force acting on 
a rigid body. It is with reference to such vectors that the follow- 
ing definitions are framed. 

By the moment of a vector F with respect to a point is meant 
the vector 

M = r X F, 

where r is the vector drawn from to any point of the line in 
which F lies. In practice, F may be a force acting on a rigid body, 
or F may be the vector momentum, mv, of a particle. 
The moment of a couple can be expressed as 

TI X F! + r, X F 2 , 

where F D F 2 are the forces of the couple and r t , r 2 are vectors 
drawn from any point of space to any points P lt P 2 of the lines 
of action of F D F 2 , respectively. 

By the moment of a vector F about a directed line L is meant the 
vector 

M = Ma, M = a - (r X F), 

where a is a unit vector having the direction and sense of L, and 
r is the vector drawn from any point of L to any point of the line 
in which F lies. Thus if F is a force acting on a rigid body, let 
its point of application be transferred to the point P nearest to 
L, and let be the point of L nearest to F ; i.e. OP is the common 
perpendicular of L and the line of action of F. Decompose F 
at P into a force parallel to L and one perpendicular to L. The 
vector moment of the latter component at P with respect to 
is Ma. 

5. Rotation of the Axes. Direction Cosines. A transforma- 
tion from one set of Cartesian axes to a second having the same 
origin (both systems being right-handed, or both left-handed) 
is characterized by the scheme of direction cosines : 



X 

y 

z n^ n% 7i 3 fc HI w 2 



VECTOR ANALYSIS 



455 



Between the nine direction cosines there exist the following 
relations : 



mS + m 2 2 + m 3 2 = 1 
n* + n 2 2 + n 3 2 = 1 



IS + mS + 



1 



n 



+ tn 2 w 3 + n 2 n a = 
+ m^m l + n 3 n x = 
-f w,m 2 + n x n 2 = 



== 

n^j + n 2 Z 2 + n 3 i! 3 = 
JiW, + Z 2 m 2 + J 3 m s = 



m 3 n 2 



m l = n 2 Z 3 n 3 Z 2 



n 2 = Z 3 m I Z^j 



Z 3 = 



1. 



APPENDIX B 

(dij\ ^ 
~jj) = /() 

Differential equations of the form : 



where 

I. f(u) = (t*-a)(6 -*) 

or 

II.' /(w) = (w - a) (6 - tO 

and ^ (w) is continuous and positive in the interval 

a ^ u ^ bj 
play an important role in Mechanics. Let us study their integrals. 

CASE I. A particular integral of (1) is found by extracting 
the square root : 

du 



and separating the variables : 

du 



dt = 



< 2 > '-Ajsr 



a ^ u ^ b. 



Geometrically, the function on the right of (2) can be inter- 
preted as the area under the curve, 



a b 



(3) 

\ / 

w 
u The graph of the function 



FIG. 153 (4) y = V(u - a) (6 - u 

456 



A DIFFERENTIAL EQUATION 



457 



is represented by Fig. 153. The reciprocal of an ordinate of this 
curve gives the corresponding ordinate of the graph of the func- 
tion (3), Fig. 154 : 

/r\ .. _ m 

V(u-a)(b -u)t(u) 

The area under the curve (5), shaded in 
the figure, represents the integral (2), or: v 



(6) t 



r du_ 

~~ J V^-~Mb~^ 



Thus this area expresses t and brings out 
the fact that t increases as u increases. 
Conversely, u increases as t increases. 
Let A be defined by the equation : 




a u b 

FIG. 154 



(7) 



r du^ 

J V(1T^~ci)(6~- 




Then the graph of u, regarded as a func- 
tion of t y 



(8) 



u = 







FIG. 155 



is as shown in Fig. 155. Its slope is at 
each extremity and positive in between. 
The definite integral, (2) or (6), has now served its purpose. 
It has yielded for a restricted interval, 

^ t g A, 

a particular solution of (1). 

Continuation by Reflection. Reflect the graph of the func- 
tion (8), Fig. 155, in the axis of ordinates, and let the curve thus 
obtained define a continuation of the function ^(0 throughout 
the interval A ^ t rg 0. Analytically the reflection is repre- 
sented by the transformation : 



Thus 



= *(- 0, 



-A 



458 APPENDIX B 

The extended function : 



is seen to satisfy the differential equation 



fdu\ 

(w) = 



Hence the function <p(t) thus defined in the interval ( A, A), or 
u = <*(0, - A ^t ^ A, 

is a solution of (1). 

To complete the definition of <p(f) for all values of t, i.e. 
oo < t < oo, we could repeat the process of reflection, using 

next the lines / = A and t = A ; 

anc * so on ' ^ ut ** * s s ^ m P^ er to 
! /i\ introduce the idea of periodicity. 



\ 



v 




Periodicity. Let the function 



now be extended to all values 
of t by the requirement of peri- 



-2A -A 

FIG. 156 odicity . 

(9) <f>(t + 2A) = <p(f), - oo < t < oo. 

Then we have one solution of Equation (1). 

The General Solution. The general solution of Equation (1) in 
the present case can now be written in the form : 

(10) u = <p(t + 7), 
where 7 is an arbitrary constant. Observe that 

(U) *>(- = <f>(i). 

Hence 

/i o\ '/ t\ ft\ 

To an arbitrary value u of u such that a < w < 6 there 
correspond two and only two values of t in the interval ( A, A), 
for which 

(13) U Q = ^>(0, 

namely 

If w = , there is only one value, namely, t = 0; and if 
w = &, then t A y A. But only one should be counted, 



A DIFFERENTIAL EQUATION 459 

since the fundamental interval of periodicity should be taken as 
an open interval, 

c <t g c + 2A or c g t < c + 2A, 

where c is arbitrary. Moreover, du/dt has opposite signs in J 
and t' Q , because of (12). 

We can now prove that there is a solution of the given differ- 
ential equation, which corresponds to arbitrary initial condi- 
tions : u = u l9 t = t 19 provided merely that 

a g H! ^ 6. 

Suppose that it is known from the physics of the problem that 
du/dt is negative initially. Now, set U Q = ^ and determine 
t Q as above so that 

w = ^(a *'(*o) <0. 

Finally, define 7 by the equation : 

*i + 7 = t Q , 7i = <o - 'i- 

Thus 7 = 7i is uniquely determined and the function 
(14) u *( + 7i) 

is the solution we set out to obtain. 

But is this solution unique, or are there still other solutions 
which satisfy the same initial conditions? If a < u^ < 6, the 
answer is affirmative for values of t near ^ ; but for remote values, 
the question of singular solutions arises, to which we now turn. 

Singular Solutions. The given differential equation admits, 
furthermore, singular solutions. The functions 

u = a, u = 6 

are obviously solutions of the differential equation : 

(15) 

each being considered in any interval for t, finite or infinite. Such 
a solution, moreover, may be combined with a solution (10) at 
any point. The solution now may follow (10) indefinitely; or 
it may switch off on a singular solution again. 

These solutions do not, however, have any validity in the 
problems of mechanics, for which the above study has been made. 
The mechanical problems depend each time on differential equa- 



460 APPENDIX B 

tions of the second order, and these have unique solutions, depend- 
ing on the initial or boundary conditions. Equation (14) repre- 
sents an integral of these equations. But the converse is not 
true, namely, that every integral of (15) is an integral of the 
second order equations why should it be ? We see, then, 
that we may be on dangerous ground when we replace the latter 
equations, in part, by the integral of energy, for example ; since the 
modified system may have solutions other than that of the given 
mechanical problem. Cf. the Author's Advanced Calculus, p. 349. 
Does this remark not call into question the validity of the 
treatment in Chap. XV, since the equation : 



is essentially the integral of energy? Not if we apply that method 
as set forth in the text. For in a suitably restricted region there 
is only one solution yielded by those methods, and we were careful 
to point out that it is the analytical continuation of this solution 
that yields the solution of the mechanical problem beyond this 
region. Thus the singular solutions are automatically eliminated. 

CASE II. This case : 



(16) (J~J = (u - a) (6 - u)*t(u), 

is more easily dealt with. A particular integral of (16) is given 
by the formula 

(17) t = f- (b _ dM === , a ^ u < b 

a 

The inverse function, 

(18) u = *>(0, ^ t < oo, 

represents an integral of (16) in the interval indicated. And 
now this solution can be completed by the definition : 

(19) <p(- t) = <p(t). 

Thus we have one solution : 
u = b (20) u = ,(<), 

oo < t < oo. 

It is now shown as before that 
the general solution is 




A DIFFERENTIAL EQUATION 461 

(21) u = ?( + 7). 

A further case, namely : 

(22) 



can be treated in a similar manner; or, more simply, be thrown 
back on the case just considered by a linear transformation. 
Finally, the case (not mentioned above) : 



(23) 

breaks up into the two distinct equations : 

a) - = + (u - a) (6 - t)vV(tt); 

b) f t =-(u-a)(b-u)Vt(d. 

Each of these is solved at once by a quadrature. 

FURTHER STUDY OF CASE I. There is another treatment of 
Case I which brings out the important fact that the function <p(t) 
is essentially a sine or cosine function : 

(24) u = C cos + C', 

where 0, in the simplest case, is proportional to the time : 

* = j<, 

and in the general case is of the form : 



where h (/) is periodic with the period 2A : 
h(t + 2A) = h(t). 

This method, moreover, may simplify the computation in case 
it is desired to tabulate the function (p(t). 
The given differential equation : 

(25) 



462 



APPENDIX B 



can be reduced by a linear transformation : 

, 2u - a - 6 
U= b-a ' 

to the form, after dropping the accent : 
(26) 

Make the substitution : 

(27) u = cos 6, < < IT. 

Equation (26) becomes, on suppressing the factor * sin 2 : 

(28) 

This equation is equivalent to the two equations : 

(29) 



(30) = 

The solution of (30) is obtained from the solution of (29) by 
changing the sign of t. 

A particular solution of (29) is given by the quadrature : 



(3D 

Write 
(32) 
where 
(33) 



9 

"/: 



de 

^(cosfl)' 



- oo <e < oo. 



f . d9 - 24. 
_J V^(cose) 

Then g(6) is periodic with the period 2v. For, 

(34) 




* In so doing we suppress the singular solutions of (26). 



A DIFFERENTIAL EQUATION 463 

But the value of the integral, because of the periodicity of the 
integrand, is 2A for all values of 0. Hence 

(35) g(e + 2r) 
Equation (31), or its equivalent, 

(36) t = ^ + 

defines 6 as a single- valued function of t, since the integral (31) 
represents a monotonic function of 0. Let be written in the 
form: 

(37) 0= J + /KO- 

Then h(t) has the period 2 A : 

(38) h(t + 2A) = h(t). 

For, let have an arbitrary value in (36) and let the correspond- 
ing value of t be t : 



Let = + 27r, and let t' be the new value of t : 

,,*('. + 20 + , ( ,. + ar) . 
By virtue of (35), 



or t' = < + 24. 

From (37) we now infer : 



Hence 



and the proof is complete. 
If we multiply (36) by v and (37) by A and add, we find : 

(39) 0()+AA(0 =0. 



464 APPENDIX B 

We are now ready to express u in terms of /. In Equation (27) 
B was restricted. Now, set generally : 

(40) 

This function is seen by direct substitution to be a solution of (26). 
If we denote it by <p(f) y the general solution of (26) will be : 

(41) u = *>(* + 7). 

The other equation, (30), leads to the same result. 

If it is a question actually of computing h(t), then the integral 
(31) can be tabulated for values of from to TT, the reckoning 
being performed by the ordinary methods for evaluating definite 
integrals Simpson's Rule, etc. 

Integral of a Periodic Function. Let f(x) be a continuous peri- 
odic function : 

f(x + A) = /(*), - oo < x < oo, 

where A is a primitive period, corresponding to 2 A above. Let 

A 

c = 





Then 

J + A 



Jf(x)dx. 



L 

f(x) dx = C, 



where x is arbitrary. For, 

X + A 

//(*) dx = f(x + A)- /(*) = 0. 
Let 

X 

/V 
f(x)dx - jx. 

c 

Then <p(x) is periodic : 

<p(x + A) = <p(x). 
For, 

x+A 

v(x + A) - *(x) = ff(x)dx -( x + A)+ 



A DIFFERENTIAL EQUATION 465 

Hence 



where X = C/A. The result may be stated as follows. 

THEOREM. The integral of a periodic function is the sum of a 
periodic function and a linear function : 



where 
and 



A 

C=ff(x)dx, X = |- 





Instead of the linear function \x we may write 
Xz + 7 or X(z - x n ), 

the function <p(x) being changed by an additive constant. In 
particular, X = if and only if 

A 

ff(x)dx = 0. 
o 



APPENDIX C 
CHARACTERISTICS OF JACOBI'S EQUATION 

Although Jacobi's partial differential equation of the first order : 

AN 
A) 



has played an important role in the solution of Hamilton's Equa- 

tions : 

rn d( Jr _ dH dp r _ m 

*> ~dt~Wr ~dt~~Wr' r-l,..-,m, 

where // = H(q ly - , q m , p ly , p m , t), we have not found it 
necessary to refer to the theory of characteristics, partly because 
we have sought certain explicit solutions by means of ingenious 
devices (separation of variables, for example) ; partly because, 
when we have needed an existence theorem, it was supplied at 
once by reference to the Cauchy Problem. Nevertheless it is 
of interest for completeness to connect the equation with its 
characteristics. 

1. The Analytic Theorem. Consider the general partial dif- 
ferential equation of the first order : 



T .. . 

L l ' ' n > > ' dx 

Let F(x ly - - , x n , z, 2/i, , 2/n), together with its partial deriva- 
tives of the first two orders, be continuous for those values of the 
arguments for which (x l9 , x n , z) is an interior point of an 
(n + l)-dimensional region * R of the space of the variables 
(x 19 , x n , z), and the yk are wholly unrestricted. Use the 
notation : 

/i\ y __ dF 7 __ dF v 3F 

(1) Xk ~^' Z -~te> Yk ~^ 

At a given point A : (a,, , a n , c, b 19 , b n ) = (a, c, b) of R 
let the Yk not all vanish ; in particular, let Y n ^ 0. 

* R shall not include any of its boundary points. 

466 



CHARACTERISTICS OF JACOBFS EQUATION 467 

The characteristic strips are defined by the system of 2n ordinary 
differential equations : 

II dxk = dz = """ dyk k = l 

Y k S y k Y k X k + y k Z* ' ' 

The solution of II. shall go through the point (x, 2, y Q ), which 
shall lie in the neighborhood of A and moreover on the manifold 

F = 0, or 

F (x x z v '2/^^=0 

Although there are 2n + 1 initial values the (2, 2, y) 
there is only a 2n-parameter family of solutions of II., for we 
may without loss of generality set x n = a n once for all. The 
solution of II. can now be written in the form : 

T. = f-(r -r . r 7 11 11 ^ 
^t ^ i \^n , -^i , , -^n 1) * 9 Ml 9 9 if* /9 

i = l,---,n-l; 

(2) 



Along any curve (2) the function F(x lt , x n , z, y^ , y n ) 
is constant, since 

dF = % X k dx k + Zcfe +5) y*d*- 

On subjecting dxk, dz, dy k to the conditions imposed by II. it 
appears that dF = 0. Hence 

(3) F(x l9 ,x n ,z,y l ,.-,y n )=C 

is an integral of the system of differential equations II. 
Characteristic strips are curves (2) for which 

(4) F(x, - - , 4-i, On, 2, 2/i, , ) = 0, 

i.e. C = in (3). This equation can be solved for y n Q since 



Thus there is a (2n l)-parameter family of characteristic strips. 
Consider now the (n + l)-dimensional space of the variables 
(&!,, x ny z), in which a solution : 

(5) z = *(*!, - -,*), 



468 APPENDIX C 

of the partial differential equation I. will lie. In the (hyper-) 
plane x n = a n of this space let a manifold be defined by the 
equation : 

(6) 2 = Cdfo , ' ' , Xn-l), 

where o)(x lt , x n -\), together with its first partial derivatives, 
is continuous in the neighborhood of the point (a,, , a n ~0, 
and 

Furthermore, let 

and let y n be given by (4) or (4'). If, now, we regard the 



as n 1 independent parameters and for symmetry in notation 
set 

X n = U n , 

the first n equations (2), combined with this last equation, will 
represent a (hyper-) surface parametrically, the equation of which 
can be thrown into the form (5) by eliminating the (u lf , w n ), 
and this function (5) is a solution of the given partial differential 
equation I. Moreover it is the most general solution; i.e. any 
solution (5), such that V satisfies the above requirements of 
continuity, can be obtained in this manner.* 

This is the general theorem of the solution of I. by means of 
characteristics. We proceed to apply the result to Jacobi's 
Equation A). 

2. Jacobi's Equation. Let 

(8) ( Xr = q " y ' = Pr > r == 1, , m = n - 1 ; 
1 z=F, x n = *. 

As regards y n , we see from I. and A) that it is given by the equa- 
tion: 

(9) F ss H(x lt , x m , * , Vi, - - , 2/m, x n ) + y n = 0. 
Equations II. now take the form : 

*For the proof cf. Goursat-Hedrick, Mathematical Analysis, or the Advanced 
Calculus, Chap. XIV, p. 366. 



CHARACTERISTICS OF JACOBFS EQUATION 469 



(10) 



m i 



m 



= - dp r dy n 
d# dff 

dq r dt 



The initial values are : 

X r Q r 3 



(H) 



/7 ?/ = 7i r =s 1 . *n 

</r > Jf r Pr , r 1, , 771 , 

^o> 2/w = "" " > ^0* 

From (10) follow first Hamilton's Equations : 



(12) 



dq r 



dt dp r ' dt dq r ' 

Furthermore, by the aid of (9), 
( . dtf^m. 

\ / fit QJ J 

at ot 
and finally, since from (12) 



m. 



(14) 



dV 

dt 



= Z PrQr - 



Observe in passing that the right-hand side of (14) is the La- 
grangean Function, L : 

H + L = 5) p r q r , 

r 

and so 
(15) 



dV -L 

~- L - 



But we have anticipated the results of the general theory and 
although obtaining the facts of the case in Equations (12) ; (13), 
and (14), we have not brought out the direct testimony of the 
general theory in the present case. Let us turn back, then, to 
Equations (2) and Condition (4) or (4'). It appears that the 
solution of Equations (10) takes the form : 



(16) 



n __ / // . 

Qr Jr(J> , 

7) / (t 

Pr ~ Jn+r \f , 



-<) 
Pi 



n V 
> Q.m , ' 0> 

, <7 m , F 0) 



Pm , 



470 APPENDIX C 

where r = 1, , m = n 1 and 

(17) y = - H (<?,, , q n , Pl , -, p m , t ) 

In the case before us the functions f rt / w + r , r = 1, , m, 
arising as they do from the solution of Equations (12), do not 
depend on F , and y n Q is given by (17). Thus we have 



(18) 

V ' ' 

and also the further integral of (10), given by (9) : 
(19) 2/n = - //(ft, - , g, p,, , ?m, 0- 

But V in (16) does depend on V . It is given by (14) : 



(30) 
or 



t 

V = 

to 



So much, then, for the discussion of the solution of Equations 
II., i.e. (10). As regards now the solution of Equation I., i.e. A) : 



(21) + 

we choose w subject to the conditions under (6) : 

(22) F = cofoo, , q m ) 
and set 



n 

= 



r ' s 



3. Application. We have seen in Chap. XV, 2, that Hamil- 
ton's Equations can be solved by a contact transformation : 

/f\n\ d$ n d$ -i 

(23) Pr = w , Pr=~ W , r = l,--,m, 

which transforms the given dynamical problem into the Equilib- 
rium Problem, the solution of which is 

Q r = a r , Pr = r , r = 1, , m, 



CHARACTERISTICS OF JACOBFS EQUATION 471 

where a r , @r are arbitrary constants, wholly unrestricted so far 
as the transformed Hamiltonian Equations : 

dQ r _ Q d^-n r-1 m 

"rfT" ' ~3T~' r-l,---,m, 

are concerned. 

The demands that the function Sfa, - , q m , Q if , Q m , 
fulfil are the following. First, it must be possible to solve the 
equations : 

(24) b r = S qr (a lt , Om, a lf , ct m , t ) 
for the a r : 

(25) oj = aj , - - - , a m = a m , 

where a r = # r , 6 r = p r are an arbitrary set of initial values 
of </r, p r . 

Furthermore, S(q l9 - , </ m , 1? , a m , shall be continuous, 
together with its derivatives : 

dS dS d*S 

dq r ' dctr dq r doL 8 ' 

in the neighborhood of the point (a r , a r , t Q ), and 

!, ,, , , m 

Finally, the function V = S(q r , <x r , t) shall satisfy Jacobi's Equa- 
tion A). 

The proof of the existence of such a function S is given by the 
theorem of 2 by setting 

(27) cofo , - , q m ) = a^i + + <* m q m . 

For now the corresponding solution of Jacobi's Equation A) : 

(28) V = S(q ly - -,q m , a n , a w , 0, 
has the property that 



Moreover, the Jacobian determinant (26) is seen to have the value 
1, and we are through. 

We have obtained this existence theorem for the function 
by means of the theorem of 2, the proof of which is based on 



472 APPENDIX C 

characteristics. But it might equally well have been derived 
directly from the existence theorem which is usually referred to 
as Cauchy's Problem, 5 below, provided we are willing to assume 
that H(q r , p r , is analytic in the point (gv, p r , t Q ). 

4. Jacobi's Equation : H, Independent of t. Consider the 
case that H does not depend on t : 

(1) H = H(q l9 - - ,<? m , p lf - ,p m ). 

Jacobi's Equation now takes the form : 



A/ , * 

A') _ + 

We seek the special solution 

(2) V = S(q l9 -,?, -,ob,0 

defnanded in 3. 

It is possible to obtain S as follows. A solution of A') can be 
found by setting 

(3) V = - ht + W, 
where 

w = w( qi , ..-,?) 

does not depend on t. Then W will satisfy the partial differential 
equation : 

r,x v ( dW 8W\ , 

C) ff^,...,^-.,... ,__)-*. 

The derivatives of H(q l} - , q m , p l9 , p m ) with respect to 
the p r are not all 0.* Let 

* 

Then the equation 

(5) ff fe, ' ' ' , ?m, Pi, ' ' , Pm) = ft 

can be solved for p l : 

(6) Pi = x(7i, ",?, A, P2i ' Pm), 
and C) is equivalent to the equation : 

^ dW . dW dW 

c) = 



* Either because of the hypotheses of Chap. XI, 3 or because H is a positive 
definite quadratic function of the p/s. 



CHARACTERISTICS OF JACOBFS EQUATION 473 

Let 

(7) W = W( qi ,*--,q m ,h,a 2 , -,) 
be that solution of C) which reduces to 

(8) W = a>(<7 2 , , fr) 



when q l = q^. If, now, we set h = !, the desired function S 
is given by the equation : 

(9) S(q l9 , q my !,--, a, = 

- o^ + TF(ft, , q m , a l9 , a m ). 
For, 

dW 



Hence 

p r = a r , r = 2, , m, 

are a system of equations which can be solved for the a r , r = 2, 
, m, and c^ is given by (5). 
It remains to examine the Jacobian, 

Since 



(J1S\ = { 0, 

\dardq a / I 1, 

we have only to show that 



0, r ? s 

r, s = 2, , m, 

r = s 



Now, 
(12) 

x i 

is given by the equation (5) : 
Hence with the aid of (4) 



and the proof is complete. 



474 



APPENDIX C 



Summary of Results. To sum up, then : the solution of 
Hamilton's Equations B) is given by the equations : 



98 



dW 



8S 



(14) 
or 



(15) 



The a r are determined in terms of the (q, p) by the equations : 

r = 2, - - - , m ; 



(16) 



= Pr, 



The # r are now given by (15) on setting q r = q r Q and substituting 
for a r the value given by (16). 

The Function W. The total differential equations which deter- 
mine the characteristics of C) are : 



(17) 
Since 

we have 

(18) 

or 

(19) 



dq r dW -dp r 
^L 2 

Sp r Pr 8p r dq r 

m_ . 

d P r ~ 9 " 

dW 



W 



r-1, 



m. 



If ff is a homogeneous quadratic function of p M , p m , then 



(20) 



W = 2 Hdt + W Q . 



CHARACTERISTICS OF JACOBFS EQUATION 475 

6. The Cauchy Problem. Let F (xi, , x n , z, y\, , y n ) 

be analytic in the point (a, c, b) = (a 1? , a n , c, b l9 , & n ) 
and let dF/dx^ ^ there. Consider the partial differential 
equation : 

fa 2Z\ n 

,...,x n , 2 , ,..-, )=o. 

Let 



be analytic in the point (a 2 , , a n ) and let 

^( 2 , ,a n ) = c, 

^*(oa, , o) = 6*, A; = 2, , M. 
Then there exists one and only one function, 

Z = ^(Xj, - - , X n ), 

which is analytic in the point (a^ , a n ), has 
^(i, , On) = c, 
^/( a i> ' ' ' > n) == 6/, y = 1, , n, 

and satisfies the given differential equation in the neighborhood 
of the point (o 1; , a n ). 

This is the existence theorem known as the Cauchy Problem. 
Cf. Goursat-Hedrick, Mathematical Analysis, Vol. II, 446. 



APPENDIX D 
THE GENERAL PROBLEM OF RATIONAL MECHANICS 

I 
PATHS 

Consider* a system of n particles m t : (x, y^ Zi) acted on by 
forces (Xi, Yi, Zi). Their motion is governed by Newton's Law: 

A) niiXi Xi niiiji = Yi mi'Zi = Z,- 

Here are Qn dependent variables, the x,, y it z,-, X^ Y i} Z t , con- 
nected by 3n equations. The problem of motion is to find 3n 
supplementary conditions whereby these 6n variables will be 
determined as functions of the time, t, and suitable initial condi- 
tions, and to solve for these functions. Each member of the 
family which forms the solution, namely the curve : 

Xi Xi \l)) y\ y i \'/j Zi Zi \tj 

Xi = Xi(t), Yi = Yi(t), Zi = Zi(t) 
determines a curve : 

Xi = xt(t), yi = 2/ t (0, *< = *;(0 



(2) 



_ . __ . __ , 

Xi ~ ~dT' Vi ~ "df ' Zi " ~dt 



in the (6n + l)-dimensional space of the (a;,-, 2/ t -, 2, ft, ?/, , 0> 
and such a curve is called a path. Obviously the paths (2) 
stand in a one-to-one relation to the curves (1). 

The problem of motion as so formulated transcends the domain 
of Rational Mechanics. In order to restrict our attention to the 
latter field, we now lay down the further postulate which, be 
it noted, is not satisfied by certain systems which occur in nature, 
viz., certain systems in which electro-magnetic phenomena are 
present. 

* The following treatment is the result of a joint study of the problem by 
Professor Bernard Osgood Koopman and myself. 

4.76 



GENERAL PROBLEM OF RATIONAL MECHANICS 477 

POSTULATE I. DYNAMICAL DETERMINATENESS. In a given 
dynamical system, when 6n + 1 constants (x^, yi () , z t -, Xi, 7/,, z,-, J ) 
are arbitrarily assigned, not more than one path (2) exists which 
passes through this point : 



THE DOMAIN ZX Those points (#;, y i} z i} x, #;, ,-, of the 
(6n + 1) -dimensional space, through which paths pass, con- 
stitute the domain D. This domain may consist of the entire 
space, or of a region of it ; but in general neither of those things 
will be the case. It is a point set, concerning the constitution of 
which we need make no hypothesis at the present moment. It 
will be restricted by later postulates. 

THEOREM I. The variables X i} F t , Zi are uniquely determined 
in the points of D : 

Xi = Xi fa, y,, Zj, x h y it Zj, t) 

(4) Yi = Yi (x/, y,-, Zj, Xj, fa, Zj, t) 

Zi = Zi (Xj, y h Z 3 ; Xj, 7/y, Zj, /) 

where (xj, y h z it Xj, y,-, z } , t) is any point of D. 

For, through each point of D passes a path, unique in virtue 
of Postulate I. Along a given path Xi, Yi, Zi are uniquely deter- 
mined as functions of t by A). Hence Xi, Yi, Zi are uniquely 
determined at the point of D in question, but not in general in 
points not lying on Z). 

THE DOMAIN R. In the (3n + l)-dimcnsional space of the 
variables (x^ yi, z^ f) those points which participate in paths 
form a point set R, which may be described as the orthogonal 
projection on this space of the domain D. In particular R may 
consist of the whole space, or of a (3n + l)-dimensional region 
in it. But in general neither of these things will be the case. 

Let P be a point of R. To P there corresponds at least one 
path given by (2). The points (x iy y^ Zi, t) represented by the 
first line of (2), namely : 

(5) Xi = Xi (0, Vi = Vi (0, Zi = ^ (0, 
all belong to R. Hence the curve (5) lies wholly in R. 



478 APPENDIX D 

Consider an arbitrary line through P, but not perpendicular 
to the axis of t. Let its direction components be a,-, ft, 7,-, K, 
where K ^ 0. There may be a path corresponding to P, such 
that at this point 

Xi : yi : Zi = <*< : ft : 7*. 

When this is not the case, not all lines through P correspond 
to paths, and so certain relations between the direction com- 
ponents (ca, pi, 7,, K) must exist. Thus we are led to a second 
postulate. 

POSTULATE II. The direction components at points of R, to which 
paths correspond, are given by the equations : 

(6) 2} (A 3i ai + B 8i ft + C a i 7 t ) + D 8 K = 0, s = 1, , cr, 
ii 

where A 8 i, B 8i , C,, D 8 are functions* of (Xi, y l , z t , t) such that the 
rank of the matrix : 

All ' ' ' Aln Bn ' Bin Cll ' Cln 

(7) 

is <r. 
Since along a curve (5) 

i ~~ ft ~~ 7i ; ~~ K 
at the point P, it follows that 

n 

B) ^ (Ati Xi + B 8 i yi + C, Zi) + D 8 = 0, s = 1, - , <r. 

These equations form a necessary and sufficient condition for 
(, yi, Zi) if (Xi, y iy z iy x iy y it z it t) is to be a point of D. 

It may happen that the system of Equations B) (a system of 
Pfaffians) admits certain integrals : 

where the rank of the matrix : 

* Throughout the whole treatment, the continuity of the functions which enter, 
and the existence and continuity of such derivatives as it may be convenient to use, 
are assumed. 



GENERAL PROBLEM OF RATIONAL MECHANICS 479 



(8) 



is I. Since the system B) may obviously be replaced by any 
non-specialized linear combination of these equations, it is clear 
that Equations B) may be so chosen that the last I of them are : 



(9) 



dt 



= 0, 



The constants Ck come to us as constants of integration in the 
system of integrals C) of the Pfaffians B). They contribute 
toward determining the particular dynamical system we are 
defining, different choices of the Ck leading to separate dynamical 
systems. They are not to be confused with constants of integra- 
tion that are determined by the initial conditions within a par- 
ticular dynamical system. 

Holonomic and Non-Holonomic Systems. If, in particular, 
I = or, Equations B) can be replaced by Equations C) and thus 
become completely integrable. The dynamical system we are 
in process of defining is then said to be holonomic. But if there 
remain a I = /* > Equations B), which then are non- 
integrable, the system is said to be non-holonomic. Equations B) 
shall now be replaced by the first p of them, and Equations C) : 



B') 

C) 



(Aaii + B ai yi + C ai Zi) + D a = 0, a = 1, ,/*; 



= /x + I. 



II 

THE FORCES. D'ALEMBERT'S PRINCIPLE 

The force X t , Y^ Zi which acts on m is made up in general of 
a force- X' iy F', Z\ which is known in terms of z t -, y^ z t -, x iy fa, z it t, 
and of further forces XJ/, F{,-, Z/, where j = 1, 2, , p, the 
components of these latter forces being wholly or in part un- 



480 



APPENDIX D 



known. Denote the unknown components by S 19 , S K . 
Then our postulates must provide for enough known equations 
between the S's and the Xi, y^ z t -, Xi, ?/,-, 2,-, t to make possible the 
elimination of the $'s between these equations and Equations A), 
with the result that the equations thus obtained, combined with 
Equations B') and C), will just suffice to determine x if y*, z> as func- 
tions of t and the initial conditions. We proceed to the details. 

D'ALEMBERT'S PRINCIPLE 

In practice the equations which the Si, , S K satisfy are 
usually linear. Our problem shall be restricted to systems which 
obey the following postulate. 

POSTULATE III. The force Xi, Y it Z{ is the sum of two forces: 

(10) 'Xi = xi + A7, Yi = y; + 17; Zi = z; + z;, 

where X\, FJ, Z\ are known in terms of the coordinates a:,-, y^ z,-, 
Xi, ilij Zi, t f an arbitrary point of D, ami where 

(11) ijxrfc + rrih. + z; $-, = (> 

i=l 
for all fi, r/i, f,- such that 

(12) 2J Abb + Shu + C'pift = 0, j8 = 1,- - , i/. 

i=l 

Here, A' ai , B' a i, C^i are known functions of the above #,-, 7/ t -, z^ 
Xi 9 tit* *i) t> an d the rank of the matrix : 



(13) 



v. Conversely, when Equations (12) are satisfied. Equation (11) 



Turning now to Equations A), we have what is known as the 
General Equation of Mechanics : 



(14) 



= 0, 



GENERAL PROBLEM OF RATIONAL MECHANICS 481 

where ,-, T/,-, f i are 3n arbitrary quantities. Under the sanction 
of Postulate III. this equation can be replaced by the following : 

(15) 2) (m t i ~ XI) fc + (m<fr - Ffl* + (w2 - Z')f - 0, 

<-l 

where ,-, ?7 t , f ,- are any 3n quantities which satisfy the condition 
(12). 

Multiply the 0-th equation (12) by X^ and subtract the re- 
sulting equation from (15) : 

(16) 2) (mtfi - X,' - 5) A'fiiljh + (mtfr - Y'< - % B'^n 

<=1 0-1 /3-1 

+ (m i z i -Z' i -^C'e i \p)t< = 0. 
0=1 

Suppose for definiteness that the determinant whose matrix 
consists of the first v columns of the matrix (13) is ^ 0. Then 
the X's can be so determined that the coefficients of the first v 
of the quantities 1, , n , i?i, - , *7n, fi, , fn in (16) will 
vanish. Substitute these values of X 1? , \ v in the remaining 
coefficients of (16). Thus a new linear equation in the ,-, 17,-, f $ - 
arises, in which only the last 3n v of these quantities appear. 
But the latter are arbitrary. Hence each coefficient must vanish. 

The 3n v equations thus obtained express the result of elim- 
inating the unknown S l , S K , i.e. the X*, Yf, Zf, from the 
problem. They contain only a?, y iy z iy Xi, #, z^ x it y iy z i} t, and 
can be written in the form : 

E) %(E yi Xi + Fyi y< + Gyi 2,) + #* = 0, 7 = 1, . , 3n - v, 

<-i 

where the coefficients E yil F yi , Gyi, Hy are known functions of 
Zt, IJi, Zi, Xi, y*, Zi, t at each point of D. 

Equations E) and B) form a necessary condition for the func- 
tions Xi(f), yi(t), Zi(t) which define a path (2). Hence if P : 
(xfj yfj Zi Q , Xi Q , yfj zP, t Q ) is an arbitrary point of Z), Equations E) 
and B) admit a solution having as its initial values the coordinates 
of JP . Furthermore, by virtue of Postulate I., this solution is 
unique. We have now arrived at a complete analytical formula- 
tion of the problem, for we can retrace our steps. Let 



482 APPENDIX D 



be a curve lying on C) and satisfying B'). Then a) gives rise to a 
curve T which lies on D. Consequently all the coefficients in B'), 
(12), and E) are determined in the points of a). Let a) also 
satisfy E). 

Since E) holds, it follows that X D , X, can be determined so 
as to make each parenthesis in (16) vanish. Next, determine 
X* 9 Yi f Z* from these X's by the equations : 



X* = 2* Afii X/3, Y* = j Bfii Xj3, Z* = j Cfti X/3. 

0=1 /3=i 0=1 

These quantities satisfy (11) and (12). On substituting them in 
(10), values of Xt, F, Z{ are obtained for which A) is true, because 
each parenthesis in (16) vanishes, and so T is a path. But there 
is only one path through an arbitrary point P of D. Hence a) is 
unique. 

Retrospect. These Postulates complete the formulation of the 
class of problems in Rational Mechanics which we set out to 
isolate. The role which d'Alembert's Principle * plays is two- 
fold. First, it requires that the relations between the unknown 
S\, ' m 9 &* shall b e linear. Secondly, it performs the elimination 
by a technique such that the multipliers {,-, T/;, f can always be 
interpreted as virtual displacements of the system of particles m : 
(xt, yi, Zi) by setting 

(17) bXi = fc byt = ??i, bZi = ft. 

Remark. In general there is no relation between the coefficients 
A 9 i, B 9i , C 8 i of Equations B) and the Ap it B^i, C'^ of Equa- 
tions (12). Hence the virtual displacements to,-, 6r/, fai of (17) 
will not coincide save as to infinitesimals of higher order with any 
possible displacement A# t , Ay iy As* due to an actual motion of the 
system in time A/. 

In a sub-class of cases it happens, however, that the 4, J3, t , Ci 
in B) and the Apt, B' ftiy C'pi in (12) are respectively equal to each 

* Historically d'Alembcrt's Principle took its start in the assumption of a con- 
dition, necessary and sufficient, that a system of forces, acting on a system of 
particles, be in equilibrium, namely, that the virtual work corresponding to a 
virtual velocity be nil. When a system of forces not in equilibrium acts on a system 
of particles, the former can be replaced by a system of forces in equilibrium 
through the introduction of "counter effective forces" or "forces of inertia" 
(sic), and thus d'Alembert arrived at the General Equation of Dynamics. 



GENERAL PROBLEM OF RATIONAL MECHANICS 483 

other. But even so, if the D a are not all 0, the virtual displace- 
ment will not tally save as to infinitesimals of higher order with 
any possible actual displacement. 

Finally it can happen that, in addition, the D, are all 0. 
Then the virtual displacement corresponds to a possible displace- 
ment. But this is a very special, though highly important, case. 



Let 
(18) 



Ill 
LAGRANGE'S EQUATIONS 



', 0m, 

-, ffm, 

-,ff, 



where the rank of the matrix : 



(19) 



dq, 



is w, and where, moreover, the region of the (x, y^ z, 0-space 
which corresponds to the points (q ly , q m , f) in which /, ??,, ^i 
are defined, at least includes the points of R. 
Let T denote the kinetic energy : 



Then, for an arbitrary choice of the q r , since 



T goes over into a function of g r , q rt t : 

T = T(q r ,q r ,t). 

Conversely, if , ^, , are any set of numbers for which these 
equations are true, the q r are uniquely determined. 



484 APPENDIX D 

Consider a path (2). Since the points # = Xi(t), yi = yi(t), 
Zi = Zi (0 all lie in R, a curve of the (q r , 0-space is thus defined : 

(20) qr = q r (t), r = 1, ...,m. 

For the path in question we have : 



__ 

dtdqr Sq r ~ Q " ' 

where 

8xi 4- Y 8yi 4- 7 8z 

<+ i+ 



Equations (21) are always true under the foregoing restrictions. 
They will be sufficient to determine the motion if the system is 
holonomic and if 



(22) 

r = 1, , m. For then 



' dXi - dyi - ' dzr 
" 



and thus Q r is known first, in terms of x<, y^ z lt x iy y iy z iy t, and 
so finally in terms of q r , q r , t. That Equations (21) can be solved 
for q l9 , q m follows from the fact that T is a positive definite 
quadratic form in the q ly , q m . 

This means in terms of the foregoing treatment that a suitable 
choice of the multipliers ,, 7? t , f t in Equation (12) is : 



\ 



vhere the 8q r are arbitrary. Equations C), if present, are all 
satisfied identically when the Xi, y^ Zi are expressed in terms of 
tte q r and t by Equation (18). " Equations B') are not present in the 
problem. The system is, to be sure, holonomic, but it is not the 
only case in which this is so. 

The General Case. We assumed in Postulate III. that X' t , F{, Z( 
are flee from the /S's, and that the S's coincide with the 
X*, Yf) Z*. We now divide the S's into two categories : 

t) a sub-set, denoted anew by Xf, F*, Z*, which fulfil the 
former requirements (11), (12), (13); 



GENERAL PROBLEM OF RATIONAL MECHANICS 485 



ii) a second sub-set, R 19 , R T > on which the XI, Y( 9 Z\ shall 
now depend linearly. 
Thus Equation (21) holds, where Q r is given by (23). Let 

(25) Q r = Qr + Q?, r = 1, - -, m, 

where Q' r is known in terms of such values of q r , q rj t as correspond 
to points of D. 

In the particular case before us, namely, Equations (18), it 
can happen that the equation : 

(26) Qi* *-! + + Qi * = 

is true for all values of the multipliers ir r for which the following 
equations hold : 

(27) Oft! T t + - - - + a'tmKm = 0, = 1, , v l9 

where n'p r depends on values of q r , q r , t, which correspond to points 
of D, and the rank of the matrix : 

/ 

(28) 

is v l ' 9 and conversely, when Equations (27) hold, then (26) is true. 
Equations B'), C) go over in the present case into : 

Bq) al*ll 4" " " " ~T~ ttam^wt ~f" &a == 0, Oi == 1, ', /Zj 9 

Cq) <&k (fir) == T*k) k = 1, * * ', lu 

where ^ ^ n ; ^ g Z, and where the rank of the matrix : 

(29) 

is /z t ; the rank of the matrix : 

(30) 

Fg~ 

being ^. 



486 APPENDIX D 

Finally it can happen that the R v , R r can be eliminated 
between these equations, thus leaving a system of equations be- 
tween the q rj qr, q r - Such a system yields a unique solution, cor- 
responding to each path of the dynamical system with which we 
set out. Thus the dynamical problem is completely formulated by 
means of Lagrange's Equations. 

All of the foregoing assumptions are in tentative form " It 
may happen " At the one extreme, the choice of the functions 
fit 9* ti can always be made so that all these things do happen ; 
for the q r can, in particular, be identified with the x i} y i} z< : 



At the other extreme, m may be chosen so small that Equations 
(21), though true, will contain unknown functions which cannot 
be eliminated namely, the R lt , R T . This means that, for 
such' a choice of the functions (18), the t -, rj f , f t - as given by 
(24) are too restricted. The &, rj if f. of Equations (11) are quan- 
tities which must be able to take on every set of values which 
satisfy (12). The .-, 77,-, {* which here figure, given by (24), are 
not free under the condition (24), but arc unwarrantably restricted 
by (24). 

In a given problem the desideratum usually is, to choose m as 
small as possible, subject to the requirement that the same degree 
of elimination of the'S's through (24) shall have been attained, 
as if Equations (11) and (12) had been used. 

IV 

NOTES 

Consider the dynamical system that consists of a bead sliding 
on a fixed circular wire and acted on by no other forces than the 
reaction of the wire. Equations A) take the form : 
mx = X, my = Y, mz = Z. 

Let the wire be a circle whose axis is the axis of 2. Then Equa- 
tions B) become : 

xx + yy = 



B) o 

This system of Pfaffians is completely integrable : 
f x 2 + 2/ 2 = a 2 
I z = c 



GENERAL PROBLEM OF RATIONAL MECHANICS 487 

Different values of the constants of integration, a and c, give 
different systems of paths, (2) ; but a path of one such system 
has no point in common with a path of a second system. 

Proceeding to the forces we see that Z = 0, since 3 = 0, and 
so we have a two-dimensional problem. 

The Smooth Wire. Assume first that the wire is smooth. Then 
the reaction is along the inner normal. 

X = X*, Y = Y*, 

and 

X*+ F% = 
provided 

^ + y t] = 0. 

Turning to Lagrange's Equations we set m = 1 and take 

x = a cos #, y = a sin q. 
Then 



= X* (- a sin ?) + 7* (a cos ?) 
= ;T(-2/) + F** = 0. 
Hence, finally : 



and it remains merely to integrate this differential equation. 

The Rough Wire. Suppose, however, the wire is rough. Let 
q > 0. Then 

X* = R cos q + pR sin q 

Y * = R sin q pR cos q. 
Lagrange's Equation : 

Jt ~dij ~ ~dq * Q' 
is still true. But 



488 APPENDIX D 

(a result at once obvious) and Lagrange's Equation becomes : 



We have not enough equations to solve the problem. This is 
the case in which Lagrange's Equations are said to "fail" or be 
"inapplicable." The failure lies, not in Lagrange's Equations, 
but in a misuse of them. We should take m = 2. Let us first 
treat the problem, however, by the methods of Parts I., II., before 
Lagrange's Equations were introduced in Part III. Here, then, 

r7 2 rr 

m = X* = - R cos B + R sin 
at* 

m-j% = F* =-juftcos0 - Rsin0. 
ut 

Equation (11) now takes the form : 

x** + 7*77 = 0, 

or 

( R cos + p,R sin 6) + (- nR cos 6 - R sin 0) rj = 0, 

or, finally, 

( x + y) + ( MZ - y) v = 0, 

and this is the form of Equation (12). Hence we may take 
= IJLX + y, rj =- x + ny. 

On substituting these values in the General Equation of 
Dynamics we have : 

/ \ d 2 x , t . ^ d?y ~ 
(i*x + V)-fc + (-x + /iy) ~ = 0. 

This equation and Equation C), namely : 

x* + y* = a 2 , 

provide us with two equations for determining x and y as functions 
of I, and thus the problem is reduced to a purely mathematical 
problem in differential equations. Observe, however, that the 
virtual displacement used in this solution : 



GENERAL PROBLEM OF RATIONAL MECHANICS 489 

is not one which is compatible with the constraints, i.e. the circular 
wire even save as to infinitesimals of higher order than e. It 
corresponds to a displacement along a line at right angles to the 
resultant of R and pR. 

Turning now to Lagrange's Equations let us choose q l and q z 
as the polar coordinates of the mass m. Then Lagrange's Equa- 
tions (21) become : 



(31) 

7<S 

Now, Equations C q ) here become : 
C fl ) r = a. 

On the other hand Equation (26) : 

here becomes : 

0, 



and thus Equation (27) takes the form : 

*"l + M^2 = 0- 

If, then, we set : 

TTi = /i, ^2 

Equations (31) and C q ) yield : 

dO* , d*0 

-. ma _ 7ri + ma _ 

or 

#8 <W 



and it remains merely to integrate this equation. 

As a further illustration of the use and abuse of Lagrange's 
Equations may be mentioned the Ladder Problems of pages 322 
and 323. 



INDEX 



Absolute unit of force, 52 

of mass, 79 
Absolute value, 24 
Acceleration, 50, 52, 287 

d'entrainement, 288 

of gravity, 56 

Vector, 90 

Addition of vectors, 4 
d'Alembert's Principle, 345, 480 
Angle of friction, 10 
Angular velocity, Vector, 170, 285 
Appell, 225, 244, 246, 307, 337 
Areas, Law of, 108 
Atwood's machine, 134 
Axes, Principal, of a central quadric, 
194, 196 

Rotation of the, 454 

B 

Bending, K , 226 

Centre of, 234 

Billiard ball, with slipping, 143, 237, 
314 

without slipping, 145, 240, 314 
Blackburn's pendulum, 184 
Bocher, 334 
Bolza, 372, 375 
Brah6, Tycho, 115 



Centripetal force, 102 
Centrodes, 159 

Space and Body, 174 
Change of units, 76 
Characteristics of Jacobi's Equation, 

466 

Charlier, 437 
Check of dimensions, 79 
Coefficient of friction, 10 

of restitution, 271 
Component of force, 2 

of velocity, 87 
Compound pendulum, 130 
Cone, Body, Space, 213 
Conservation of energy, 256 
Conservative field of force, 255, 258 
Constrained motion, 95 
Constraint, Forces of, 315, 325 
Contact transformations, 390, 399 

Particular, 403 
Coordinates, Cyclic, 430 

Generalized or intrinsic, 297 

Normal, 335 
Coriolis, 288 
Couples, 25, 29, 34, 37 

Composition of, 31 

Nil, 31 

Resultant of n, 31 

Vector representation of, 38 
Cyclic coordinates, 430 



Canonical equations, 338, 395 

transformations, 389 
Carathe'odory, 381, 445 
Cart wheels, 241, 314 
Cauchy problem, 475 
Central force, 108, 379, 427, 434 
Centre of bending, 234 
Centre of gravity, 26, 27, 42 

Motion of the, 120 
Centre of mass, Motion of the, 

123 
Centrifugal force, 101 

field of force, 106, 291 

oil cup, 105 



5, Definition of, 356 

Critique of, 379 
Dancing tea cup, 165 
Decomposition of force, 2 
Dimensions, Check of, 79 
Direction cosines of the moving axes, 

216, 454 
Dyne, 56 

120, E 

Elastic strings, 58 
Elasticity, Perfect, 272 
Electromagnetic field, 254 
Ellipsoid of inertia, 192 
491 



492 



INDEX 



Energy, Kinetic, 75, 260 

Conservation of, 256 

Potential, 255 

Work and, for a rigid body, 266 
Equation, Solution of a trigonomet- 
ric, 12 

Fundamental, 367 

of moments, cf . Moments 
Equilibrium of couples, 31 

of a dynamical system, 330 

of forces in a plane, 32 

of forces in space, 36, 41 

of n forces, 9 

of three forces, 5 

of a rigid body, 26 

Problem, 413 
Escalator, 265 
Euler's Angles, 214, 215 

Dynamical Equations, 210, 325, 
352 

Equations, 359 

Geometrical Equations, 214 



Field of force, 253 

Centrifugal, 291 

Gravitational, 254 

Electromagnetic, 254 
Force, 1 

Absolute unit of, 52, 55 

Central, 108, 379, 427, 434 

Centrifugal, 101, 291 

Centrifugal field of, 291 

Centripetal, 102 

Component of, 2 

of constraint, 315, 325 

Equilibrium of three, 5, 43; cf. 
Equilibrium 

Field of, 253 

function, 253 

Moment of a, 28 

Parallel, in a plane, 21 ; in space, 36 

Parallelogram of, 2 

Polygon of, 7 

Triangle of, 4 
Foucault Pendulum, 292 
Friction, 9 

Angle of, 10 

Coefficient of, 10 

Problems in, 19 
Function, Lagrangean, 338 

Hamiltonian, 342 
Fundamental equation, 367 



Generalized coordinates, 297 
Geodesies, 308 
Goursat, 468 

Gravitation, Motion under the attrac- 
tion of, 69 

Law of universal, 116 
Gravitational constant, 116 
Gravity, Acceleration of, 56 
Gyration, Radius of, 129 
Gyroscope, 217 

Intrinsic treatment of the, 225 

H 

Hadamard, 224 

Hamilton's Canonical Equations, 338, 
395 

Proof of, 342 

Solution of, 410, 432 

Reduction of, to the Equilibrium 
Problem, 411, 413 

for constant energy, 411, 420 
Hamiltonian Function, 342 
Hamilton's Principle, 371 

Integral, 356 

Integral a minimum, 381 
Harmonic Motion, Simple, 64, 415 
Haskins, 228 
Hedrick, 468 
Helical motion, 168 
Hertz, 244 
Holder, 370 
Holonomic, 313, 479 
Hooke's Law, 59, 74 
Huntington, 208 
Huygens, 133 



Impact of particles, 270 

Oblique, 274 

of rigid bodies, 277 
Impulse, 271 
Inertia, 118 

Ellipsoid of, 192 

Moment of, 128, 137, 191 

Product of, 191 
Instantaneous centre, 154, 157, 160 

axis, 168, 173 
Integral invariants, 392 
Integral of kinetic energy, 362 

of a periodic function, 464 

of rational mechanics, 360 



INDEX 



493 



Internal work, 258 

Intrinsic treatment of the gyroscope, 

225 

coordinates, functions, 297 
equations of the gyroscope, 236 

Invariable line and plane, 201 

Inverse problem, 114 

Isolate the System, 102 



Jacobi's Equation, 410, 468, 472 
Characteristics of, 466 
Integral a minimum, 386 
Principle of Least Action, 377 



K , bending, 226 
Rater's pendulum, 133 
Kemble, 234, 263 
Kepler's laws, 115 
Kinetic energy, 75 

of a rigid system, 166, 260 

Integral of, 362 
Klein-Sommerfeld, 236, 246 
Koopman, 123, 476 
Kreisel, 236, 246 



Ladder, 147, 322, 323, 353 
Lagrange's Equations, 299, 304, 312, 
348, 350, 482 

multipliers, 194, 316, 375 

Principle of Least Action, 374, 377 

Solution of, Equations, 326 
Lagrangean function, 338 
Lagrangean integral, 372 
Lagrangean integral a minimum, 381 
Lagrangean system, 338 
Law of areas, 108 

of nature, 109, 116 

of universal gravitation, 116 

of work and energy, 258 
Least Action, 374, 377 
Leval, Turbine of, 247 
Lissajou's curves, 182, 190 

M 

Mass, Absolute unit of, 79 
Moments about centre of, 139, 205 
Motion of the centre of, 120, 201 
Notion of, 118 



Material point, 50 
Maxwell, 119 
Moment of a force, 28 

of a couple, 29 

of a vector, 37 

of a localized vector, 197 

of momentum, 197, 205 

of inertia, 128, 137, 191 

Theorem of Moments, 127, 200 

Moments about the centre of mass, 
139, 205 

Moments about the instantaneous 
centre, 207 

Moments about an arbitrary point, 
205, 208 

of a vector about a line, 40 
Momentum, 50, 201, 350 

Moment of, 197, 200, 350 
Motion under the attraction of gravi- 
tation, 69 

Newton's Laws of, 50 

Simple Harmonic, 64, 415 

Constrained, 95 

Simple Pendulum, 97 

Spherical Pendulum, 306 

in a resisting medium, 81 

in a plane and in space, 86 

of a projectile, 93, 424 

on a smooth curve, 99 

on a space curve, 100 

of the centre of gravity, 120 

of space, General case of, 175 

about a fixed point, 212 
Moving axes, 172, 216 

curve, 299 

surface, 303 

N 

Newton's Laws of Motion, 50 

Second Law, 92, 290 
Non-holonomic, 244, 313, 479 
Normal, 9 

Principal, 90 
Normal coordinates, 335 
Nul vector (or nil vector), 5, 447 

couple, 31 
Numerical value, 24 



Operator, Symbolic vector, 254 
Orbit of a planet, 111, 113, 435 
Oscillations, Small, 333 
Osculating plane, 90, 92 



494 



INDEX 



Parabolic motion, 93 

Parallel forces in a plane, 21, 23 

in space, 36 

Parallelogram of forces, 2 
Particle, 50 
Pendulum, Blackburn's, 184 

Compound, 130 

Foucault, 292 

Rater's, 133 

Simple, 97, 419 

Spherical, 306 

Torsion, 139 
Periodic time, 111 
Perturbations, 440 
Poincar6, 392 
Poinsot, 213 
Potential, 253 

energy, 255 
Poundal, 56 
Principal axes of a central quadric, 

194 

Principle of the motion of the centre 
of mass, 123 

of moments, 139 

of moments with respect to the 
centre of mass, 205 

d'Alembert's, 345, 480 

Hamilton's, 371 

of Least Action, 374 

Variational, 370 
Product of inertia, 191 
Projectile, Motion of a, 93, 424 



Quadric, Central, 194 



Radius of gyration, 129 
Eankine, 10 
Rectilinear motion, 49 
Relative velocities, 177 
Resistance, Graph of the, 84 
Resisting medium, Motion in a, 81 
Resultant, 2 

of parallel forces in a plane, 21, 23 

of n couples, 31, 36 

of n forces in a plane, 32 

of n forces in space, 36, 38 

axis, 39 

of two velocities, 87 
Riemann, 381, 445 



Rotation of the axes, 454 
about a fixed axis, 127, 136 
of a plane lamina, 139 
of a rigid body, Chap. VI 

Routh, 134, 202, 225, 246, 337 

Ruled surfaces, 176 

S 
<r, 197 

Evaluation of, for a rigid system. 
208 

Transformation of, 202 
Sabine, 190 
Sand tunnel, 185 
Ship's stabilizer, 236, 247 
Simple Harmonic Motion, 64, 415 
Simple pendulum, 97, 419 
Small oscillations, 333 
Smooth curve, 99 

Solution of trigonometric equation, 
12 

Hamilton's Equations, 410, 432 
Sommerfeld, 236, 246 
Space curve, Motion on a, 100 
Spherical pendulum, 306 
Stabilizer, Ship's, 236, 247 
Stationary, 359 
Strings, Elastic, 58 
Symbolic vector operator, 254 



Tautochrone, 98 

Tennis ball, 282 

Top, 220, 438 

Torque, 29 

Torsion pendulum, 139 

Transformation of <r, 202 

Contact, 390, 399, 413 

Canonical, 389 

of Hamilton's Equations by con- 
tact transformations, 400, 413 
Translation, 159 
Transmissibility of force, 22 
Triangle of forces, 4 
Trigonometric equation, 12 

theorem, 44 

Two body problem, 114, 879, 427, 434 
TychoBrah6, 115 
Tyndall, 166 



Units, Absolute, 52, 55, 79 
Change of, 76