ANALYTICAL DYNAMIcs.—The fundamental principles of dynamics, and their application to special problems, are explained in the articles MECHANICS and MOTION, LAWS OF, where brief indications are also given of the more general methods of investigating the properties of a dynamical system, independently of the accidents of its particular constitution, which were inaugurated by J. L. Lagrange. These methods, in addition to the unity and breadth which they have introduced into the treatment of pure dynamics, have a peculiar interest in relation to modern physical speculation, which finds itself confronted in various directions with the problem of explaining on dynamical principles the properties of systems whose ultimate mechanism can at present only be vaguely conjectured. In determining the properties of such systems the methods of analytical geometry and of the infinitesimal calculus (or, more generally, of mathematical analysis) are necessarily employed; for this reason the subject has been named Analytical Dynamics. The following article is devoted to an outline of such portions of general dynamical theory as seem to be most important from the physical point of view.
1. General Equations of Impulsive Motion.
The systems contemplated by Lagrange are composed of discrete particles, or of rigid bodies, in finite number, connected (it may be) in various ways by invariable geometrical relations, the fundamental postulate being that the position of every particle of the system at any time can be completely specified by means of the instantaneous values of a finite number of independent variables
gz,•••q,,, each of which admits of continuous variation over a certain range, so that if x, y, z be the Cartesian coordinates of any one particle, we have for example
x=f(qi, y=&c., z=&c., . . (I)
where the functions f differ (of course) from particle to particle. In modern language, the variables q1, q2,...q„ are generalized coordinates serving to specify the configuration of the system; their derivatives with respect to the time are denoted by q1, gz,•••gn, and are called the generalized components of velocity. The continuous sequence of configurations assumed by the system in any actual or imagined motion (subject to the given connexions) is called the
path.
For the purposes of a connected outline of the whole subject it is convenient to deviate somewhat from the historical order of Impulsive development, and to begin with the consideration of motton. impulsive motion. Whatever the actual motion of the
system at any instant, we may conceive it to be generated instantaneously from rest by the application of proper impulses. On this view we have, if x, y, z be the rectangular coordinates of any particle m,
mi=X', my=Y', mz=Z', . . (2)
where X', Y', Z' are the components of the impulse on m. Now let Sx, by, Sz be any infinitesimal variations of x, y, z which are consistent with the connexions of the system, and let us form the equation
Em(iSx+ySy+zaz)=Z(X'Sx+Y'Iy+Z'Sz), . (3) where the sign E indicates (as throughout this article) a summation extending over all the particles of the system. To transform (3) into an equation involving the variations Sq1, Sq2,••• of the generalized coordinates, we have
x= a4ig+q2+..., &c., &c. .
Sx=— ql+a4~Sqz+..., &c., &c., . aqi and therefore
Em(iSx+yIy+z&z) =Augi+Ai2g2+...)Sqi +(A21gi+A22g2+.••)Sq2+•••,
where
Arr=Zm (ax 2+ (aqr/ 2+ \aqr/ 2 l
A„=Em ax ax ay ay azaz =A I (7)
OD. aqs+aqr aqs+aqr aq, J
If we form the expression for the kinetic energy T of the system, we find
2T=fm(i2+y2 +22) =A11g12 +A22422 +... +2Al2g1g2 +... (8)
The coefficients An, A22,...Al2,... are by an obvious analogy called the coefficients of inertia of the system; they are in general functions of the coordinates qi, 42,.... The equation (6) may now be written
m(iax+ysy+zaz) =aq —OD + 442+ (9)
This may be regarded as the cardinal formula in Lagrange's method. For the righthand side of (3) we may write
Z(X'Sx+Y'Sy+Z'Sz) =Q'ibgi+Q'2Sg2+ (io) where
Q'r=~(X, ax+Y, ay+Z, az\ . (II)
aqr aqr aqr
The quantities Qi, Q2, • . are called the generalized components of impulse. Comparing (9) and (1o), we have, since the variations Sqi, Sq2,... are independent,
aT=Q'1, aT=Q'2 ... (12)
a4i aqz
These are the general equations of impulsive motion. It is now usual to write
pr=aq (13)
The quantities Pi, P2,... represent the effects of the several component impulses on the system, and are therefore called the generalized components of momentum. In terms of them we have
~ni(tIx+yay+zaz) =piagi+P2Sg2+... (i4)
Also, since T is a homogeneous quadratic function of the velocities 41, q2...,
2T=pigi+P242+ ••. • (i5)
This follows independently from (14), assuming the special variations Sx=idt, &c., and therefore SQ1g1dt, SQ2=g2dt,... .
Again, if the values of the velocities and the momenta in any other motion of the system through the same configuration be distinguished by accents, we have the identity
p1q'1+p2q'2+ ••• =p'141+p'242+...1 . (16) each side being equal to the symmetrical expression
Angiq'i +A22424'z+... +Al2(414'2+4'142) +••• (i7)
The theorem (16) leads to some important reciprocal relations. Thus, let us suppose that the momenta pi, p2,... all vanish with
the exception of p1, and similarly that the momenta P'i, p'z,... all vanish except p'z. We have then piq'i=p'z4z, or
qz: pi=q'1: p'z.. (18)
The interpretation is simplest when the coordinates qi, qz are both of the same kind, e.g. both lines or both angles. We may then conveniently put Pi =P'2, and assert that the velocity of the first type due to an impulse of the second type is equal to the velocity of the second type due to an equal impulse of the first type. As an example, suppose we have a chain of straight links hinged each to the next, extended in a straight line, and free to move. A blow at right angles to the chain, at any point P, will produce a certain velocity at any other point Q; the theorem asserts that an equal velocity will be produced at P by an equal blow at Q. Again, an impulsive couple acting on any link A will produce a certain angular velocity in any other link B ; an equal couple applied to B will produce an equal angular velocity in A. Also if an impulse F applied at P produce an angular velocity w in a link A, a couple Fa applied to A will produce a linear velocity wa at P. Historically, we may note that reciprocal relations in dynamics were first recognized by H. L. F. Helmholtz in the domain of acoustics; their use has been greatly extended by Lord Rayleigh.
The equations (13) determine the momenta p1, p2,... as linear functions of the velocities q2,••• . Solving these, we can express qi, q2,..• as linear functions of Pi, A"... The resulpng Velocities equations give us the velocities produced by any given interms ol system of impulses. Further, by substitution in (8), momenta. we can express the kinetic energy as a homogeneous
quadratic function of the momenta pi, p2,.... The kinetic energy, as so expressed, will be denoted by T' ; thus
2T' =A'11p12+A'22p22+•••+2A'12pP2+... . (i9)
where A'11, A'22, ••• A'12,... are certain coefficients depending on the configuration. They have been called by Maxwell the coefficients of mobility of the system. When the form (19) is given, the values
. (6)
Reciprocal theorems.
of the velocities in terms of the momenta can be expressed in a remarkable form due to Sir W. R. Hamilton. The formula (15) may be written
p141+p242+...=T+T, (20)
where T is supposed expressed as in (8), and T' as in (19). Hence if, for the moment, we denote by S a variation affecting the velocities, and therefore the momenta, but not the configuration, we have
p1S41 +41SP+p2S42+42Sp2+... = OT T' aT. aT aT' aT'
_ Sq1+84Sq2+... +aplplSplM p2Sp2+.... In virtue of (13) this reduces to
aT' aT'
41Sp1+42sp2+... =ap1Sp'+ap2Sp2+....
Since Bpi, 432,... may be taken to be independent, we infer that
aT' aT'
41=v, 42=dp2'
In the very remarkable exposition of the matter given by James Clerk Maxwell in his Electricity and Magnetism, the Hamiltonian expressions (23) for the velocities in terms of the impulses are obtained directly from first principles, and the formulae (13) are then deduced by an inversion of the above argument.
An important modification of the above process was introduced by E. J. Routh and Lord Kelvin and P. G. Tait. Instead of expressRouth's ing the kinetic energy in terms of the velocities alone, modifica or In terms of the momenta alone, we may express it in
tion. terms of the velocities corresponding to some of the co
ordinates, say qi, q2,..•q,., and of the momenta corresponding to the remaining coordinates, which (for the sake of dis
tinction) we may denote by x, x', x",.... Thus, T being expressed as a homogeneous quadratic function of ql, 42,••.g„., X, the momenta corresponding to the coordinates x, x', x",••• may be written
aT, aT " aT
aX' IC =—71 IC =aX", ... (24)
These equations, when written out in full, determine X, X', i",••• as linear functions of 41, K, K', K", .. We now consider the function
— K Y— (25)
supposed expressed, by means of the above relations in terms of gl g2i... K, K, K",.... Performing the operation S on both sides of (25), we have
a R
ag S41+... I aKSK+...=='ki+...+.=5X+...
KaiXSK—..., (26) where, for brevity, only one term of each type has been exhibited. Omitting the terms which cancel in virtue of (24), we have
aR . aR aT.
a,8g1+...+aK SK+...=a41bg1+...xSK (27) Since the variations Sq,, Sq2,... Sq,,,, SK, SK, SK",... may be taken to be independent, we have
aT aR aT aR
__
pl a41 (TT: P2_a42=aQ2' •." (28)
aR , aR " aR
and x=—dK' x =—aK' X = (29)
—aK ....
An important property of the present transformation is that, when expressed in terms of the new variables, the kinetic energy is the sum of two homogeneous quadratic functions, thus
T = 6+K, . . . . (30) where 6 involves the velocities 41, 42,... 4m alone, and K the momenta K, K', K",... alone. For in virtue of (29) we have, from (25),
aR ,aR 'aR
T =R (KaK +K UK +K lK+...) . (31) and it is evident that the terms in R which are bilinear in respect
of the two sets of variables 41, 42,... 4m and K, K",... will dis
appear from the righthand side.
It may be noted that the formula (30) gives immediate proof of two important theorems due to Bertrand and to Lord Kelvin Maximum respectively. Let us suppose, in the first place, that and the system is started by given impulses of certain types, minimum but is otherwise free. J. L. F. Bertrand's theorem is to
energy. the effect that the kinetic energy is greater than if by
impulses of the remaining types the system were constrained to take any other course. We may suppose the coordinates to be so chosen that the constraint is expressed by the vanishing of the velocities 41, q2,•.• q>n, whilst the given impulses are K, K', K",... IIence the energy in the actual motion is greater than in the constrained motion by the amount 6.
Again, suppose that the system is started with prescribed velocity components qi, q2,... 4, , by means of proper impulses of the corresponding types, but is otherwise free, so that in the motion actually generated we have K=o, K'=o, K"=o,... and therefore K=o. The kinetic energy is therefore less than in any other motion consistent with the prescribed velocityconditions by the value which K assumes when K, K, K",... represent the impulses due to the constraints.
Simple illustrations of these theorems are afforded by the chain of straight links already employed. Thus if a point of the chain be held fixed, or if one or more of the joints be made rigid, the energy generated by any given impulses is less than if the chain had possessed its former freedom.
2. Continuous Motion of a System.
We may proceed to the continuous motion of a system. The equations of motion of any particle of the system are of the form
m=X, nzy=Y, mz=Z . . . (I)
Now let x+Sx, y+Sy, z+Sz be the coordinates of m in any Lagrange, arbitrary motion of the system differing infinitely little equations. from the actual motion, and let us form the equation
Em(xSx+ySy+Sz) =E(XSx+YSy+ZSz) . (2)
Lagrange's investigation consists in the transformation of (2) into an equation involving the independent variations Sql, Sq2,... Sq,.
It is important to notice that the symbols S and d/dt are commutative, since
Sx =a (x+Sx) ai =atsx, &c.
Hence
d
Em(2ox+yoy+i8z) =atEm(J x+ySy+HSz)
— Em(xSx+ySy+at)
d =dt(p1Sg1+p2Sg2+...)—ST, .
by § 1 (14). The last member may be written P1Sg1 +p1S41+P2Sg2 +P2642+...
aT aT aT aT —a41Sq'—Q Sqi—aQSg2—aQ"Sg2—... (5)
Hence, omitting the terms which cancel in virtue of § I (13), we find
Im(zox+ysy+zHz) _ (Pi —a4) Sgi+ (1)2 —OQ2) 15q2+.... (6) For the righthand side of (2) we have
Z(XSx+YSy+ZSz) =Qlsg1+Q26g2+
where Q, = (Xag+1'aq +Za4) . (8)
The quantities Qi, Q2,... are called the generalized components of force acting on the system.
Comparing (6) and (7) we find
aT aT P1—al=Q1, p2aQ2=Q2, ...,
or, restoring the values of pl, P2,••.,
d aT aT d aT OT
dt (aQ1) —aq1= Ql, 7it (a42) a  =Q2' Q2,
These are Lagrange's general equations of motion. Their number is of course equal to that of the coordinates ql, q2,... to be deterrnined.
Analytically, the above proof is that given by Lagrange, but the terminology employed is of much more recent date, having been first introduced by Lord Kelvin and P. G. Tait; it has greatly promoted the physical application of the subject. Another proof of the equations (Io), by direct transformation of coordinates, has been given by Hamilton and independently by other writers (see MECHANICS), but the variational method of Lagrange is that which stands in closest relation to the subsequent developments of the subject. The chapter of Maxwell, already referred to, is a most instructive commentary on the subject from the physical point of view, although the proof there attempted of the equations (to) is fallacious.
In a " conservative system " the work which would have to be done by extraneous forces to bring the system from rest in some standard configuration to rest in the configuration (qi, q2,... q,.) is independent of the path, and may therefore be regarded as a definite function of ql, q2,... q,. Denoting this function (the potential energy) by V, we have, if there be no extraneous force on the system,
Z(XSx+YSy+ZSz) _ . . . (II)
and therefore
av aV
Q1 =  j1' Q2 = aQ2..
(21) (22)
(23)
(3) (4)
(7)
• (9)
(to)
758
Hence the typical Lagrange's equation may be now written in the form
d aT aT aV
d CT) _aqr = aqr'
pr = — ,
j—(V—T). (14)
It has been proposed by Helmholtz to give the name kinetic potential to the combination V—T.
As shown under MECHANICS, § 22, we derive from (10)
ddt =Q1g1+Q242+ (15) and therefore in the case of a conservative system free from extraneous force,
dt(TfV) =0 or T+V =const., . (16) which is the equation of energy. For examples of the application of the formula (13) see MECHANICS, § 22.
3. Constrained Systems.
It has so far been assumed that the geometrical relations, if any, which exist between the various parts of the system are of the type § I (I), and so do not contain t explicitly. The extension of Lagrange's equations to the case of " varying relations " of the type
x=.f(t, qi, g2,...gn), y=&c., z=&c., was made by J. M. L. Vieille. We now have
Ox ax . ax.
x=at+aglgl+aQ242+..., &c., &c., (2)
ax=aglSQlaQ2Sg2+., &c., &c., . (3) so that the expression § I (8) for the kinetic energy is to be replaced by
2T=ao+2ai41+2a242+••.+An412+A22422+...+Al24142+..., (4) where
ao = zm (at) 2+ (i) 2+ (at) 2
ax ax ay ay Oz az tt
`,. _ Zm at aqr+at aqr+at aqr
and the forms of Arr, A,. are as given by § I (7). It is to be remembered that the coefficients ao, a1, a2, ...An, A22,... Al2... will in general involve t explicitly as well as implicitly through the coordinates qi, g2.... Again, we find
F.m(xSx+ysy+2Sz) = (al+A11 1+Al242+...)&qi
+ (a2+Az141+A2242+...)aq2+...
OT, q1+aq
= Sq2+..
=pAbg1+p2Sg2+ (6) where p,. is defined as in § I (13). The derivation of Lagrange's equations then follows exactly as before. It is to be noted that the equation § 2 (15) does not as a rule now hold. The proof involved the assumption that T is a homogeneous quadratic function of the velocities 41, 42....
It has been pointed out by R. B. Hayward that Vieille's case can be brought under Lagrange's by introducing a new coordinate (x) in place of t, so far as it appears explicitly in the relations (I). We have then
2T=a.42+2(a142+a242+...)x+A11412+A22422+...+2Al24142+.... (7)
The equations of motion will be as in § 2 (TO), with the additional equation
and dt{{I+m(x2+y2)}+m(xy—yx)]=I.. . . (13)
If we suppose adjusted so as to maintain ¢=o, or (again) if we suppose the moment of inertia I to be infinitely great, we obtain the familiar equations of motion relative to moving axes, viz.
m(2—2wy—w2x) =X, m(/+2wx—w2y) =Y, mz=Z, . (14)
where co has been written for 4. These are the equations which we should have obtained by applying Lagrange's rule at once to the formula
2T =m(x2+y2+z2)+2mw(xy—y±)+mw2(x2+y2), . (15)
which gives the kinetic energy of the particle referred to axes rotating with the constant angular velocity w. (See MECHANICS, § 13.)
More generally, let us suppose that we have a certain group of coordinates x, x', x",••. whose absolute 'values do not affect the expression for the kinetic energy, and that by suitable forces of the corresponding types the velocitycomponents X, X', X",••• are maintained constant. The remaining coordinates being denoted by q1, qz,... q,,, we may write
2T=6+To+2(a141+a242+•••)Ji+2(x'141+x242+•••)X +..., (16)
where is a homogeneous quadratic function of the velocities 41, 4z,•..Qn of the type §i (8), whilst To is a homogeneous quadratic function of the velocities k, X , i",••• alone. The remaining terms, which are bilinear in respect of the two sets of velocities, are indicated more fully. The formulae (Io) of § 2 give n equations of the type
d a6 aro aTo
di aqr aqr+(r, 1)41+(r, 2)42+...aqr =Qr (17)
where
Aar act..
aa'r Oa',
(r, s) _ (aqa— aqr ) x+ (aqg aqr z'+....
These quantities (r, s) are subject to the relations
(r, s) _ — (s, r), (r, r) =o. (19)
The remaining dynamical equations, equal in number to the coordinates x, x', x", yield expressions for the forces which
must be applied in order to maintain the velocities z, i",••• constant; they need not be written down. If we follow the method by which the equation of energy was established in § 2, the equations (17) lead, on taking account of the relations (19), to
a(6—To)=QIgl+Q242+... Qngn,.
or, in case the forces Qr depend only on the coordinates q1, q2,..•q„ and are conservative,
6+V —To = cont. . . . (21) The conditions that the equations (17) should be satisfied by zero values of the velocities 41, 42,...4.
are
&To Qr=aqr,
or in the case of conservative forces
i.e. the value of V —To must be stationary.
We may apply this to the case of a system whose configuration relative to axes rotating with constant angular velocity ((a) is defined by means of the n coordinates qi,
q ,...q,.
This is important on account of its bearing on the kinetic theory of the tides. Since the Cartesian coordinates
x, y, z of any particle m of the system relative to the moving axes are functions of qi, q2,...q,,, of the form § i (I), we have, by (15)
26=Em(.x2+2+22), 2To=w2Em(x2+y2), (24)
a, = Em (Hay —yax) (25)
agr aqr '
(r, s) =2w.Zma
ax, y
,g 4* (26)
The conditions of relative equilibrium are given by (23).
It will be noticed that this expression V—To, which is to be stationary, differs from the true potential energy by a term which represents the potential energy of the system in relation to fictitious " centrifugal forces." The question of stability of relative equilibrium will be noticed later (§ 6).
It should be observed that the remarkable formula (20) may in the present case be obtained directly as follows. From (15) and (14) we find
a =(6+To)+w.Zm(xyyx) =dt(6To)+w.Z(xYyX). (27)
(13)
or, again,
Case of varying relations.
(I)
d aT_aT=X, (8) dt az ax
where X is the force corresponding to the coordinate x. We may suppose X to be adjusted so as to make x=o, and in the remaining equations nothing is altered if we write t for x before, instead of after, the differentiations. The reason why the equation § 2 (15) no longer holds is that we should require to add a term Xi on the righthand side; this represents the rate at which work is being done by the constraining forces required to keep constant.
As an example, let x, y, z be the coordinates of a particle relative to axes fixed in a solid which is free to rotate about the axis of z. If 42 be the angular coordinate of the solid, we find without difficulty
2T =m(x2+y2+22)+2cim(xy—y±)+{I+m(x2+y2)}0, . (9) where I is the moment of inertia of the solid. The equations of motion, viz.
d aT aT d aT aT d aT aT I dr a`x —ax =X, d ay —ay =Y, at a  Oz =Z, (o)
d aT aT dta ad) 43, .
and
become
m(—2 y—x0—y4i)=X, m(/+2c—yci2+xci)=Y, mz=Z,(12)
(18)
(20)
(22) (23)
Rotating axes.
whence
This must be equal to the rate at which the forces acting on the system do work, viz. to
wE(xYyX)+Q1g1+Q2g2+ ••• +Q4.,
where the first term represents the work done in virtue of the rotation.
We have still to notice the modifications which Lagrange's equations undergo when the coordinates qi, q2,•••q, are not all independently variable. In the first place, we may suppose them connected by a number m ( x",••.then being the angular coordinates of the gyrostats relatively to their frames. Again, in theoretical hydrodynamics we have the problem of moving solids in a frictionless liquid ; the ignored coordinates x, x', x" , ••. then refer to the fluid, and are infinite in number. The same question presents itself in various physical speculations where certain phenomena are ascribed to the existence of latent motions in the ultimate constituents of matter. The general theory of such systems has been treated by E. J. Routh, Lord Kelvin, and H. L. F. Helmholtz.
If we suppose the kinetic energy T to be expressed, as in Lagrange's method, in terms of the coordinates and Routh', the velocities, the equations of motion corresponding equations. to x, x', x", . reduce, in virtue of the above hypotheses, to the forms
d aT=o d aT _~ d aT
d OX aX =o , , d aX
whence
aT aT , aT (2)
X =K, K, aX,l=K , where K, K', K", .. are the constant momenta corresponding to the
cyclic coordinates x, x', .... These equations are linear in x, x', X", • . ; solving them with respect to these quantities and substituting in the remaining Lagrangian equations, we obtain m differential equations to determine the remaining coordinates qi, q2, ... qm• The object of the present investigation is to ascertain the general form of the resulting equations. The retained coordinates q1, Q2, ... q+n may be called (for distinction) the palpable coordinates of the system; in many practical questions they are the only coordinates directly in evidence.
If, as in § I (25), we write
R=T—KX—K'X'—K"X"—..., (3) and imagine R to be expressed by means of (2) as a quadratic function of Qt, q2, •.. 4m, K, K', K", ... with coefficients which are in general functions of the coordinates q1, q2, ..• q,, then, performing the operation S on both sides, we find
OR, . aR OR aT aT
aQ1g1 +...+ as SK+... +ag1Q1Sg1+... = aQ1og1+...+aQ1bg1+... aT aT
+aXSX+...+aX1Sg1+...—KSX—XSK—.... (4)
Constrained
systems.
. (I)
(3)
(5) . (6)
• (7)
the case of
aH OH
41=apt, q2=ap2, •••r
. (II) . (12)
(I)
760
Omitting the terms which cancel by (2), we find aT aR aT aR
4941=4941 4942 =aye, .. ,
aT aR aT OR
4941=aQ1, 4942 =aq2, ... ,
OR , aR " aR
X = aK, X =a ,, X =aK",...
Substituting in § 2 (to), we have
daR aR daR aR
dt aql aql =Q' ' dt 494 aq2 =Q2, ...
These are Routh's forms of the modified Lagrangian equations. Equivalent forms were obtained independently by Helmholtz at a later date.
The function R is made up of three parts, thus
R=R2,0+R1,1+R02, . . (9)
where R;,o is a homogeneous quadratic function of 41, 42,...4m, Ro,2 is a homogeneous quadratic function of x, K, K",..., whilst R1,1 consists of products of the velocities 41, 42,..4. into the momenta K, x', K".... Hence from (3) and (7) we
T=R— (Ka +K~R+K"a +...)
= R2,o — R0,2.
If, as in § t (30), we write this in the form T=+K,
then (3) may be written
R = IJ y R R
 K+$141+$242+..., (I2)
where $1, $2,... are linear functions of K, K', K",..., say
Nr = a,.K+a',K'+ere' +.. . (13)
the coefficients as, a„ a",,... being in general functions of the coordinates q1, q2,... q,,. Evidently $r denotes that part of the momentumcomponent aR/494, which is due to the cyclic motions. Now
d OR =d (ate+$r) —d a +494"41+aRr42+ (14)
dt dt a4r dt a a 1 aq2
OR 496 OK 49$1. al%.
aqr =aqr —aqr +agrgl +agrg2+...
Hence, substituting in (8), we obtain the typical equation of motion of a gyrostatic system in the form
d O6 a6
d a a+ (r, 1)11+(r, 2)42+...+(r, s)4e+...+asKr =Qr, (16)
where
4949, OS,
(r, s) =a—q..—a
ag a4.. (17)
This form is due to Lord Kelvin. When q1, q2,... gm have been determined, as functions of the time, the velocities corresponding to the cyclic coordinates can be found, if required, from the relations (7), which may be written
aK
x = aK 4914149242...,
aK hh X'=aK 49'141a'212 ...,
&c., &c.
It is to be particularly noticed that
(r, r) = o, (r, s) = — (s, r). . . (19)
Hence, if in (16) we put r=1, 2, 3,... m, and multiply by 41, 42,... 4m respectively, and add, we find
dt(6+K) =Q141+Q242+..., or,'in the case of a conservative system
6+V+K=cont., . . (21)
which is the equation of energy.
The equation (16) includes § 3 (17) as a particular case, the eliminated coordinate being the angular coordinate of a rotating solid having an infinite moment of inertia.
In the particular case where the cyclic momenta K, IC', K",... are all zero, (16) reduces to
dam a~
dt 494, aqr =Qr.
The form is the same as in § 2, and the system now behaves, as
regards the coordinates q1, q2,... q,,,, exactly like the acyclic type
there contemplated. These coordinates do not, however, now
fix the position of every particle of the system. For example, if
by suitable forces the system be brought back to its initial con
figuration (so far as this is defined by q1, q2,... q,,), after performing
any evolutions, the ignored coordinates x, x', x",... will not in general return to their original values.
If in Lagrange's equations § 2 (to) we reverse the sign of the timeelement dt, the equations are unaltered. The motion is therefore reversible; that is to say, if as the system is passing through any configuration its velocities qi, q2,... qm be all reversed, it will (if the forces be the same in the same configuration) retrace its former path. But it is important to observe that the statement does not in general hold of a gyrostatic system; the terms of (16), which are linear in 41, q2,... change sign with dt, whilst the others do not. Hence the motion of a gyrostatic system is not reversible, unless indeed we reverse the cyclic motions as well as the velocities 41, q2,... D.. For instance, the precessional motion of a top cannot be reversed unless we reverse the spin.
The conditions of equilibrium of a system with latent cyclic motions are obtained by putting q1=o, q2=o,... ¢,,,=o in (16); viz. they are
aK aK
Q1 =a—Q1, Q2 =aq2
These may of course be obtained independently. Thus if the system
be guided from (apparent) rest in the configuration (ql, q2,... q,,,)
to rest in the configuration (gi+Sg1, q2+Sg2,...q,,,+sqm), the work done by the forces must be equal to the increment of the kinetic energy. Hence
(Mgr +Q2642+... =SK, . (24)
which is equivalent to (23). The conditions are the same as for the equilibrium of a system without latent motion, but endowed with potential energy K. This is important from a physical point of view, as showing how energy which is apparently potential may in its ultimate essence be kinetic.
By means of the formulae (18), which now reduce to
aK , aK " aK
X = .aK , X =49K , x =ale, (25)
K may also be expressed as a homogeneous quadratic function of the cyclic velocities x, X', X,.... Denoting it in this form by To, we have
S(To+K) =25K =S(KX+K )'c'+K"X"+...) . . (26)
Performing the variations, and omitting the terms which cancel by (2) and (25), we find
aTo_ aK aTo OK
49Q1 — 49g1' 4942 — 4942,
so that the formulae (23) become
aTo aTo
Q1=—4941, Q2=—aQ2, (28)
A simple example is furnished by the top (MECHANICS, § 22). The cyclic coordinates being 4, we find
2—A92, 2K=(a—v cos fi)2 v2
A sin 2B +C '
2To=A sin2B +C(~+ cos 0)2, . (29) whence we may verify that aT0/00= —aK/a0 in accordance with (27). And the condition of equilibrium
aK aV 4949 =00
gives the condition of steady precession.
6. Stability of Steady Motion.
The small oscillations of a conservative system about a configuration of equilibrium, and the criterion of stability, are discussed in MECHANICS, § 23. The question of the stability of given types of motion is more difficult, owing to the want of a sufficiently general, and at the same time precise, definition of what we mean by "stability." A number of definitions which have been propounded by different writers are examined by F. Klein and A. Sommerfeld in their work Uber die Theorie des Kreisels (18971903). Rejecting previous definitions, they base their criterion of stability on the character of the changes produced in the path of the system by small arbitrary disturbing impulses. If the undisturbed path be the limiting form of the disturbed path when the impulses are indefinitely diminished, it is said to be stable, but not otherwise. For instance, the vertical fall of a particle under gravity is reckoned as stable, although for a given impulsive disturbance, however small, the deviation of the particle's position at any time t from the position which it would have occupied in the original motion increases indefinitely with t. Even this criterion, as the writers quoted themselves recognize, is not free from ambiguity unless the phrase ",limiting form," as applied to a path, be strictly defined. It appears, moreover, that a definition which is analytically precise may not in all cases be easy to reconcile with geometrical prepossessions. Thus a particle moving in a circle about a centre of force varying inversely as the cube of the distance will if slightly disturbed either fall into the centre, or recede to infinity, after describing in either case a spiral with an infinite number of
. (8)
Kelvin's equations.
have
. (15)
. (20)
. (22)
Kinetostatics.
. (23)
• (27)
. (30)
convolutions. Each of these spirals has, analytically, the circle as its limiting form, although the motion in the circle is most naturally described as unstable.
A special form of the problem, of great interest, presents itself in the steady motion of a gyrostatic system, when the noneliminated coordinates qi, q2, ... q,0 all vanish (see § 5). This has been discussed by Routh, Lord Kelvin and Tait, and Poincare. These writers treat the question, by an extension of Lagrange's method, as a problem of small oscillations. Whether we adopt the notion of stability which this implies, or take up the position of Klein and Sommerfeld, there is no difficulty in showing that stability is ensured if V+K be a minimum as regards variations of qi, qz,... q„,. The proof is the same as that of Dirichlet for the case of statical stability.
We can illustrate this condition from the case of the top, where, in our previous notatiom,
z z
V+K=MghcosO+(2Asin B +2C' (I)
To examine whether the steady motion with the centre of gravity vertically above the pivot is stable, we must put u = v. We then find without difficulty that V+K is a minimum provided v2>_4AMgh. The method of small oscillations gave us the condition v2>4AMgh, and indicated instability in the cases v2c4AMgh. The present criterion can also be applied to show that the steady precessional motions in which the axis has a constant inclination to the vertical are stable.
The question remains, as before, whether it is essential for stability that V+K should be a minimum. It appears that from the point of view of the theory of small oscillations it is not essential, and that there may even be stability when V+K is a maximum. The precise conditions, which are of a somewhat elaborate character, have been formulated by Routh. An important distinction has, however, been established by Thomson and Tait, and by Poincare, between what we may call ordinary or temporary stability (which is stability in the above sense) and permanent or secular stability, which means stability when regard is had to possible dissipative forces called into play whenever the coordinates qi, q2,... q,, vary. Since the total energy of the system at any instant is given (in the notation of § 5) by an expression of the form 6+V+K, where 5 cannot be negative, the argument of Thomson and Tait, given under MECHANICS, § 23, for the statical question, shows that it is a necessary as well as a sufficient condition for secular stability that V+K should be a minimum. When a system is " ordinarily " stable, but " secularly " unstable, the operation of the frictional forces is to induce a gradual increase in the amplitude of the free vibrations which are called into play by accidental disturbances.
There is a similar theory in relation to the constrained systems considered in § 3 above. The equation (21) there given leads to the conclusion that for secular stability of any type of motion in which the velocities qi, qz, ... 4s are zero it is necessary and sufficient that the function V—To should be a minimum.
The simplest possible example of this is the case of a particle at the lowest point of a smooth spherical bowl which rotates with constant angular velocity (w) about the vertical diameter. This position obviously possesses " ordinary " stability. If a be the radius of the bowl, and 8 denote angular distance from the lowest point, we have
V—To=mga(1—cos 0)—amw2a2 sin' 0; (2)
this is a minimum for B =o only so long as w2
End of Article: ANALYTICAL 

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