Routhian mechanics

Edward John Routh, 1831–1907.

In analytical mechanics, a branch of theoretical physics, Routhian mechanics is a hybrid formulation of Lagrangian mechanics and Hamiltonian mechanics developed by Edward John Routh. Correspondingly, the Routhian is the function which replaces both the Lagrangian and Hamiltonian functions.

The Routhian, like the Hamiltonian, can be obtained from a Legendre transform of the Lagrangian, and has a similar mathematical form to the Hamiltonian, but is not exactly the same. The difference between the Lagrangian, Hamiltonian, and Routhian functions are their variables. For a given set of generalized coordinates representing the degrees of freedom in the system, the Lagrangian is a function of the coordinates and velocities, while the Hamiltonian is a function of the coordinates and momenta.

The Routhian differs from these functions in that some coordinates are chosen to have corresponding generalized velocities, the rest to have corresponding generalized momenta. This choice is arbitrary, and can be done to simplify the problem. It also has the consequence that the Routhian equations are exactly the Hamiltonian equations for some coordinates and corresponding momenta, and the Lagrangian equations for the rest of the coordinates and their velocities. In each case the Lagrangian and Hamiltonian functions are replaced by a single function, the Routhian. The full set thus has the advantages of both sets of equations, with the convenience of splitting one set of coordinates to the Hamilton equations, and the rest to the Lagrangian equations.

Often the Routhian approach may offer no advantage, but one notable case where this is useful is when a system has cyclic coordinates (also called "ignorable coordinates"), by definition those coordinates which do not appear in the original Lagrangian. The Lagrangian equations are powerful results, used frequently in theory and practice, since the equations of motion in the coordinates are easy to set up. However, if cyclic coordinates occur there will still be equations to solve for all the coordinates, including the cyclic coordinates despite their absence in the Lagrangian. The Hamiltonian equations are useful theoretical results, but less useful in practice because coordinates and momenta are related together in the solutions - after solving the equations the coordinates and momenta must be eliminated from each other. Nevertheless, the Hamiltonian equations are perfectly suited to cyclic coordinates because the equations in the cyclic coordinates trivially vanish, leaving only the equations in the non cyclic coordinates.

The Routhian approach has the best of both approaches, because cyclic coordinates can be split off to the Hamiltonian equations and eliminated, leaving behind the non cyclic coordinates to be solved from the Lagrangian equations. Overall fewer equations need to be solved compared to the Lagrangian approach.

As with the rest of analytical mechanics, Routhian mechanics is completely equivalent to Newtonian mechanics, all other formulations of classical mechanics, and introduces no new physics. It offers an alternative way to solve mechanical problems.

Definitions

In the case of Lagrangian mechanics, the generalized coordinates q₁, q₂, ... and the corresponding velocities dq₁/dt, dq₂/dt, ..., and possibly time t, enter the Lagrangian,

$L(q_{1},q_{2},\ldots ,{\dot {q}}_{1},{\dot {q}}_{2},\ldots ,t)\,,\quad {\dot {q}}_{i}={\frac {dq_{i}}{dt}}\,,$

where the overdots denote time derivatives.

In Hamiltonian mechanics, the generalized coordinates q₁, q₂, ... and the corresponding generalized momenta p₁, p₂, ..., and possibly time, enter the Hamiltonian,

$H(q_{1},q_{2},\ldots ,p_{1},p_{2},\ldots ,t)=\sum _{i}{\dot {q}}_{i}p_{i}-L(q_{1},q_{2},\ldots ,{\dot {q}}_{1}(p_{1}),{\dot {q}}_{2}(p_{2}),\ldots ,t)\,,\quad p_{i}={\frac {\partial L}{\partial {\dot {q}}_{i}}}\,,$

where the second equation is the definition of the generalized momentum p_i corresponding to the coordinate q_i (partial derivatives are denoted using ∂). The velocities dq_i/dt are expressed as functions of their corresponding momenta by inverting their defining relation. In this context, p_i is said to be the momentum "canonically conjugate" to q_i.

The Routhian is intermediate between L and H; some coordinates q₁, q₂, ..., q_n are chosen to have corresponding generalized momenta p₁, p₂, ..., p_n, the rest of the coordinates ζ₁, ζ₂, ..., ζ_s to have generalized velocities dζ₁/dt, dζ₂/dt, ..., dζ_s/dt, and time may appear explicitly;

Routhian (n + s degrees of freedom)

$R(q_{1},\ldots ,q_{n},\zeta _{1},\ldots ,\zeta _{s},p_{1},\ldots ,p_{n},{\dot {\zeta }}_{1},\ldots ,{\dot {\zeta }}_{s},t)=\sum _{i=1}^{n}p_{i}{\dot {q}}_{i}(p_{i})-L(q_{1},\ldots ,q_{n},\zeta _{1},\ldots ,\zeta _{s},{\dot {q}}_{1}(p_{1}),\ldots ,{\dot {q}}_{n}(p_{n}),{\dot {\zeta }}_{1},\ldots ,{\dot {\zeta }}_{s},t)\,,$

where again the generalized velocity dq_i/dt is to be expressed as a function of generalized momentum p_i via its defining relation. The choice of which n coordinates are to have corresponding momenta, out of the n + s coordinates, is arbitrary.

The above is used by Landau and Lifshitz, and Goldstein. Some authors may define the Routhian to be the negative of the above definition.

Given the length of the general definition, a more compact notation is to use boldface for tuples (or vectors) of the variables, thus q = (q₁, q₂, ..., q_n), ζ = (ζ₁, ζ₂, ..., ζ_s), p = (p₁, p₂, ..., p_n), and d ζ/dt = (dζ₁/dt, dζ₂/dt, ..., dζ_s/dt), so that

$R(\mathbf {q} ,{\boldsymbol {\zeta }},\mathbf {p} ,{\dot {\boldsymbol {\zeta }}},t)=\mathbf {p} \cdot {\dot {\mathbf {q} }}-L(\mathbf {q} ,{\boldsymbol {\zeta }},{\dot {\mathbf {q} }},{\dot {\boldsymbol {\zeta }}},t)\,,$

where · is the dot product defined on the tuples, for the specific example appearing here:

$\mathbf {p} \cdot {\dot {\mathbf {q} }}=\sum _{i=1}^{n}p_{i}{\dot {q}}_{i}\,.$

Equations of motion

For reference, the Lagrangian equations for s degrees of freedom are a set of s coupled second order ordinary differential equations in the coordinates

${\frac {d}{dt}}{\frac {\partial L}{\partial {\dot {q}}_{j}}}={\frac {\partial L}{\partial q_{j}}}\,,$

where j = 1, 2, ..., s, and the Hamiltonian equations for n degrees of freedom are a set of 2n coupled first order ordinary differential equations in the coordinates and momenta

${\dot {q}}_{i}={\frac {\partial H}{\partial p_{i}}}\,,\quad {\dot {p}}_{i}=-{\frac {\partial H}{\partial q_{i}}}\,.$

Below, the Routhian equations of motion are obtained in two ways, in the process other useful derivatives are found that can be used elsewhere.

Two degrees of freedom

Consider the case of a system with two degrees of freedom, q and ζ, with generalized velocities dq/dt and dζ/dt, and the Lagrangian is time-dependent. (The generalization to any number of degrees of freedom follows exactly the same procedure as with two). The Lagrangian of the system will have the form

$L(q,\zeta ,{\dot {q}},{\dot {\zeta }},t)$

The differential of L is

$dL={\frac {\partial L}{\partial q}}dq+{\frac {\partial L}{\partial \zeta }}d\zeta +{\frac {\partial L}{\partial {\dot {q}}}}d{\dot {q}}+{\frac {\partial L}{\partial {\dot {\zeta }}}}d{\dot {\zeta }}+{\frac {\partial L}{\partial t}}dt\,.$

Now change variables, from the set (q, ζ, dq/dt, dζ/dt) to (q, ζ, p, dζ/dt), simply switching the velocity dq/dt to the momentum p. This change of variables in the differentials is the Legendre transformation. The differential of the new function to replace L will be a sum of differentials in dq, dζ, dp, d(dζ/dt), and dt. Using the definition of generalized momentum and Lagrange's equation for the coordinate q:

$p={\frac {\partial L}{\partial {\dot {q}}}}\,,\quad {\dot {p}}={\frac {d}{dt}}{\frac {\partial L}{\partial {\dot {q}}}}={\frac {\partial L}{\partial q}}$

we have

$dL={\dot {p}}dq+{\frac {\partial L}{\partial \zeta }}d\zeta +pd{\dot {q}}+{\frac {\partial L}{\partial {\dot {\zeta }}}}d{\dot {\zeta }}+{\frac {\partial L}{\partial t}}dt$

and to replace pd(dq/dt) by (dq/dt)dp, recall the product rule for differentials, and substitute

$pd{\dot {q}}=d({\dot {q}}p)-{\dot {q}}dp$

to obtain the differential of a new function in terms of the new set of variables:

$d(L-p{\dot {q}})={\dot {p}}dq+{\frac {\partial L}{\partial \zeta }}d\zeta -{\dot {q}}dp+{\frac {\partial L}{\partial {\dot {\zeta }}}}d{\dot {\zeta }}+{\frac {\partial L}{\partial t}}dt\,.$

Introducing the Routhian

$R(q,\zeta ,p,{\dot {\zeta }},t)=p{\dot {q}}(p)-L$

where again the velocity dq/dt is a function of the momentum p, we have

$dR=-{\dot {p}}dq-{\frac {\partial L}{\partial \zeta }}d\zeta +{\dot {q}}dp-{\frac {\partial L}{\partial {\dot {\zeta }}}}d{\dot {\zeta }}-{\frac {\partial L}{\partial t}}dt\,,$

but from the above definition, the differential of the Routhian is

$dR={\frac {\partial R}{\partial q}}dq+{\frac {\partial R}{\partial \zeta }}d\zeta +{\frac {\partial R}{\partial p}}dp+{\frac {\partial R}{\partial {\dot {\zeta }}}}d{\dot {\zeta }}+{\frac {\partial R}{\partial t}}dt\,.$

Comparing the coefficients of the differentials dq, dζ, dp, d(dζ/dt), and dt, the results are Hamilton's equations for the coordinate q,

${\dot {q}}={\frac {\partial R}{\partial p}}\,,\quad {\dot {p}}=-{\frac {\partial R}{\partial q}}\,,$

and Lagrange's equation for the coordinate ζ

${\frac {d}{dt}}{\frac {\partial R}{\partial {\dot {\zeta }}}}={\frac {\partial R}{\partial \zeta }}$

which follow from

${\frac {\partial L}{\partial \zeta }}=-{\frac {\partial R}{\partial \zeta }}\,,\quad {\frac {\partial L}{\partial {\dot {\zeta }}}}=-{\frac {\partial R}{\partial {\dot {\zeta }}}}\,,$

and taking the total time derivative of the second equation and equating to the first. Notice the Routhian replaces the Hamiltonian and Lagrangian functions in all the equations of motion.

The remaining equation states the partial time derivatives of L and R are negatives

${\frac {\partial L}{\partial t}}=-{\frac {\partial R}{\partial t}}\,.$

Any number of degrees of freedom

For n + s coordinates as defined above, with Routhian

$R(q_{1},\ldots ,q_{n},\zeta _{1},\ldots ,\zeta _{s},p_{1},\ldots ,p_{n},{\dot {\zeta }}_{1},\ldots ,{\dot {\zeta }}_{s},t)=\sum _{i=1}^{n}p_{i}{\dot {q}}_{i}(p_{i})-L$

the equations of motion can be derived by a Legendre transformation of this Routhian as in the previous section, but another way is to simply take the partial derivatives of R with respect to the coordinates q_i and ζ_j, momenta p_i, and velocities dζ_j/dt, where i = 1, 2, ..., n, and j = 1, 2, ..., s. The derivatives are

${\frac {\partial R}{\partial q_{i}}}=-{\frac {\partial L}{\partial q_{i}}}=-{\frac {d}{dt}}{\frac {\partial L}{\partial {\dot {q}}_{i}}}=-{\dot {p}}_{i}\,$

${\frac {\partial R}{\partial p_{i}}}={\dot {q}}_{i}\,$

${\frac {\partial R}{\partial \zeta _{j}}}=-{\frac {\partial L}{\partial \zeta _{j}}}\,,$

${\frac {\partial R}{\partial {\dot {\zeta }}_{j}}}=-{\frac {\partial L}{\partial {\dot {\zeta }}_{j}}}\,,$

${\frac {\partial R}{\partial t}}=-{\frac {\partial L}{\partial t}}\,.$

The first two are identically the Hamiltonian equations. Equating the total time derivative of the fourth set of equations with the third (for each value of j) gives the Lagrangian equations. The fifth is just the same relation between time partial derivatives as before. To summarize

Routhian equations of motion (n + s degrees of freedom)

${\dot {q}}_{i}={\frac {\partial R}{\partial p_{i}}}\,,\quad {\dot {p}}_{i}=-{\frac {\partial R}{\partial q_{i}}}\,,$

${\frac {d}{dt}}{\frac {\partial R}{\partial {\dot {\zeta }}_{j}}}={\frac {\partial R}{\partial \zeta _{j}}}\,.$

The total number of equations is 2n + s, there are 2n Hamiltonian equations plus s Lagrange equations.

Energy

Since the Lagrangian has the same units as energy, the units of the Routhian are also energy. In SI units this is the Joule.

Taking the total time derivative of the Lagrangian leads to the general result

${\frac {\partial L}{\partial t}}={\frac {d}{dt}}\left(\sum _{i=1}^{n}{\dot {q}}_{i}{\frac {\partial L}{\partial {\dot {q}}_{i}}}+\sum _{j=1}^{s}{\dot {\zeta }}_{j}{\frac {\partial L}{\partial {\dot {\zeta }}_{j}}}-L\right)\,.$

If the Lagrangian is independent of time, the partial time derivative of the Lagrangian is zero, ∂L/∂t = 0, so the quantity under the total time derivative in brackets must be a constant, it is the total energy of the system

$E=\sum _{i=1}^{n}{\dot {q}}_{i}{\frac {\partial L}{\partial {\dot {q}}_{i}}}+\sum _{j=1}^{s}{\dot {\zeta }}_{j}{\frac {\partial L}{\partial {\dot {\zeta }}_{j}}}-L\,.$

(If there are external fields interacting with the constituents of the system, they can vary throughout space but not time). This expression requires the partial derivatives of L with respect to all the velocities dq_i/dt and dζ_j/dt. Under the same condition of R being time independent, the energy in terms of the Routhian is a little simpler, substituting the definition of R and the partial derivatives of R with respect to the velocities dζ_j/dt,

$E=R-\sum _{j=1}^{s}{\dot {\zeta }}_{j}{\frac {\partial R}{\partial {\dot {\zeta }}_{j}}}\,.$

Notice only the partial derivatives of R with respect to the velocities dζ_j/dt are needed. In the case that s = 0 and the Routhian is explicitly time-independent, then E = R, that is, the Routhian equals the energy of the system. The same expression for R in when s = 0 is also the Hamiltonian, so in all E = R = H.

If the Routhian has explicit time dependence, the total energy of the system is not constant. The general result is

${\frac {\partial R}{\partial t}}={\dfrac {d}{dt}}\left(R-\sum _{j=1}^{s}{\dot {\zeta }}_{j}{\frac {\partial R}{\partial {\dot {\zeta }}_{j}}}\right)\,,$

which can be derived from the total time derivative of R in the same way as for L.

Cyclic coordinates

The Routhian formulation is useful for systems with cyclic coordinates, because by definition those coordinates do not enter L, and hence R. The corresponding partial derivatives of L and R with respect to those coordinates are zero, which equates to the corresponding generalized momenta reducing to constants. To make this concrete, if the q_i are all cyclic coordinates, and the ζ_j are all non cyclic, then

${\frac {\partial L}{\partial q_{i}}}={\dot {p}}_{i}=-{\frac {\partial R}{\partial q_{i}}}=0\quad \Rightarrow \quad p_{i}=\alpha _{i}\,,$

where the α_i are constants. With these constants substituted into the Routhian, R is a function of only the non cyclic coordinates and velocities (and in general time also)

$R(\zeta _{1},\ldots ,\zeta _{s},\alpha _{1},\ldots ,\alpha _{n},{\dot {\zeta }}_{1},\ldots ,{\dot {\zeta }}_{s},t)=\sum _{i=1}^{n}\alpha _{i}{\dot {q}}_{i}(\alpha _{i})-L(\zeta _{1},\ldots ,\zeta _{s},{\dot {q}}_{1}(\alpha _{1}),\ldots ,{\dot {q}}_{n}(\alpha _{n}),{\dot {\zeta }}_{1},\ldots ,{\dot {\zeta }}_{s},t)\,,$

The 2n Hamiltonian equations in the cyclic coordinates automatically vanish,

${\dot {q}}_{i}={\frac {\partial R}{\partial p_{i}}}=0\,,\quad {\dot {p}}_{i}=-{\frac {\partial R}{\partial q_{i}}}=0\,,$

and the s Lagrangian equations are in the non cyclic coordinates

${\frac {d}{dt}}{\frac {\partial R}{\partial {\dot {\zeta }}_{j}}}={\frac {\partial R}{\partial \zeta _{j}}}\,.$

Thus the problem has been reduced to solving the Lagrangian equations in the non cyclic coordinates, with the advantage of the Hamiltonian equations cleanly removing the cyclic coordinates.

If we are interested in how the cyclic coordinates change with time, the equations for the generalized velocities corresponding to the cyclic coordinates can be integrated.

Examples

The Routhian method does not guarantee the equations of motion will be simple, however it will lead to fewer equations.

Central potential in spherical coordinates

One general class of mechanical systems with cyclic coordinates are those with central potentials, because potentials of this form only have dependence on radial separations and no dependence on angles.

Consider a particle of mass m under the influence of a central potential V(r) in spherical polar coordinates (r, θ, φ)

$L(r,{\dot {r}},\theta ,{\dot {\theta }},{\dot {\phi }})={\frac {m}{2}}({\dot {r}}^{2}+{r}^{2}{\dot {\theta }}^{2}+r^{2}\sin ^{2}\theta {\dot {\phi }}^{2})-V(r)\,.$

Notice φ is cyclic, because it does not appear in the Lagrangian. The momentum conjugate to φ is the constant

$p_{\phi }={\frac {\partial L}{\partial {\dot {\phi }}}}=mr^{2}\sin ^{2}\theta {\dot {\phi }}\,,$

in which r and dφ/dt can vary with time, but the angular momentum p_φ is constant. The Routhian can be taken to be

${\begin{aligned}R(r,{\dot {r}},\theta ,{\dot {\theta }})&=p_{\phi }{\dot {\phi }}-L\\&=p_{\phi }{\dot {\phi }}-{\frac {m}{2}}{\dot {r}}^{2}-{\frac {m}{2}}r^{2}{\dot {\theta }}^{2}-{\frac {p_{\phi }{\dot {\phi }}}{2}}+V(r)\\&={\frac {p_{\phi }{\dot {\phi }}}{2}}-{\frac {m}{2}}{\dot {r}}^{2}-{\frac {m}{2}}r^{2}{\dot {\theta }}^{2}+V(r)\\&={\frac {p_{\phi }^{2}}{2mr^{2}\sin ^{2}\theta }}-{\frac {m}{2}}{\dot {r}}^{2}-{\frac {m}{2}}r^{2}{\dot {\theta }}^{2}+V(r)\,.\end{aligned}}$

We can solve for r and θ using Lagrange's equations, and do not need to solve for φ since it is eliminated by Hamiltonian's equations. The r equation is

${\frac {d}{dt}}{\frac {\partial R}{\partial {\dot {r}}}}={\frac {\partial R}{\partial r}}\quad \Rightarrow \quad -m{\ddot {r}}=-{\frac {p_{\phi }^{2}}{mr^{3}\sin ^{2}\theta }}-mr{\dot {\theta }}^{2}+{\frac {\partial V}{\partial r}}\,,$

and the θ equation is

${\frac {d}{dt}}{\frac {\partial R}{\partial {\dot {\theta }}}}={\frac {\partial R}{\partial \theta }}\quad \Rightarrow \quad -m(2r{\dot {r}}{\dot {\theta }}+r^{2}{\ddot {\theta }})=-{\frac {p_{\phi }^{2}\cos \theta }{mr^{2}\sin ^{3}\theta }}\,.$

The Routhian approach has obtained two coupled nonlinear equations. By contrast the Lagrangian approach leads to three nonlinear coupled equations, mixing in the first and second time derivatives of φ in all of them, despite its absence from the Lagrangian.

The r equation is

${\frac {d}{dt}}{\frac {\partial L}{\partial {\dot {r}}}}={\frac {\partial L}{\partial r}}\quad \Rightarrow \quad m{\ddot {r}}=mr{\dot {\theta }}^{2}+mr\sin ^{2}\theta {\dot {\phi }}^{2}-{\frac {\partial V}{\partial r}}\,,$

the θ equation is

${\frac {d}{dt}}{\frac {\partial L}{\partial {\dot {\theta }}}}={\frac {\partial L}{\partial \theta }}\quad \Rightarrow \quad 2r{\dot {r}}{\dot {\theta }}+r^{2}{\ddot {\theta }}=r^{2}\sin \theta \cos \theta {\dot {\phi }}^{2}\,,$

the φ equation is

${\frac {d}{dt}}{\frac {\partial L}{\partial {\dot {\phi }}}}={\frac {\partial L}{\partial \phi }}\quad \Rightarrow \quad 2r{\dot {r}}\sin ^{2}\theta {\dot {\phi }}+2r^{2}\sin \theta \cos \theta {\dot {\theta }}{\dot {\phi }}+r^{2}\sin ^{2}\theta {\ddot {\phi }}=0\,.$

Symmetric mechanical systems

Spherical pendulum

Spherical pendulum: angles and velocities.

Consider the spherical pendulum, a mass m (known as a "pendulum bob") attached to a rigid rod of length l of negligible mass, subject to a local gravitational field g. The system rotates with angular velocity dφ/dt which is not constant. The angle between the rod and vertical is θ and is not constant.

The Lagrangian is

$L(\theta ,{\dot {\theta }},{\dot {\phi }})={\frac {m\ell ^{2}}{2}}({\dot {\theta }}^{2}+\sin ^{2}\theta {\dot {\phi }}^{2})+mg\ell \cos \theta \,,$

and φ is the cyclic coordinate for the system with constant momentum

$p_{\phi }={\frac {\partial L}{\partial {\dot {\phi }}}}=m\ell ^{2}\sin ^{2}\theta {\dot {\phi }}\,.$

which again is physically the angular momentum of the system about the vertical. The angle θ and angular velocity dφ/dt vary with time, but the angular momentum is constant. The Routhian is

${\begin{aligned}R(\theta ,{\dot {\theta }})&=p_{\phi }{\dot {\phi }}-L\\&=p_{\phi }{\dot {\phi }}-{\frac {m\ell ^{2}}{2}}{\dot {\theta }}^{2}-{\frac {p_{\phi }{\dot {\phi }}}{2}}-mg\ell \cos \theta \\&={\frac {p_{\phi }{\dot {\phi }}}{2}}-{\frac {m\ell ^{2}}{2}}{\dot {\theta }}^{2}-mg\ell \cos \theta \\&={\frac {p_{\phi }^{2}}{2m\ell ^{2}\sin ^{2}\theta }}-{\frac {m\ell ^{2}}{2}}{\dot {\theta }}^{2}-mg\ell \cos \theta \end{aligned}}$

The θ equation is found from the Lagrangian equations

${\frac {d}{dt}}{\frac {\partial R}{\partial {\dot {\theta }}}}={\frac {\partial R}{\partial \theta }}\quad \Rightarrow \quad -m\ell ^{2}{\ddot {\theta }}=-{\frac {p_{\phi }^{2}\cos \theta }{m\ell ^{2}\sin ^{3}\theta }}+mg\ell \sin \theta \,,$

or simplifying by introducing the constants

$a={\frac {p_{\phi }^{2}}{m^{2}\ell ^{4}}}\,,\quad b={\frac {g}{\ell }}\,,$

gives

${\ddot {\theta }}=a{\frac {\cos \theta }{\sin ^{3}\theta }}-b\sin \theta \,.$

This equation resembles the simple nonlinear pendulum equation, because it can swing through the vertical axis, with an additional term to account for the rotation about the vertical axis (the constant a is related to the angular momentum p_φ).

Applying the Lagrangian approach there are two nonlinear coupled equations to solve.

The θ equation is

${\frac {d}{dt}}{\frac {\partial L}{\partial {\dot {\theta }}}}={\frac {\partial L}{\partial \theta }}\quad \Rightarrow \quad m\ell ^{2}{\ddot {\theta }}=m\ell ^{2}\sin \theta \cos \theta {\dot {\phi }}^{2}-mg\ell \sin \theta \,,$

and the φ equation is

${\frac {d}{dt}}{\frac {\partial L}{\partial {\dot {\phi }}}}={\frac {\partial L}{\partial \phi }}\quad \Rightarrow \quad 2\sin \theta \cos \theta {\dot {\theta }}{\dot {\phi }}+\sin ^{2}\theta {\ddot {\phi }}=0\,.$

Heavy symmetrical top

Heavy symmetric top in terms of the Euler angles.

The heavy symmetrical top of mass M has Lagrangian

$L(\theta ,{\dot {\theta }},{\dot {\psi }},{\dot {\phi }})={\frac {I_{1}}{2}}({\dot {\theta }}^{2}+{\dot {\phi }}^{2}\sin ^{2}\theta )+{\frac {I_{3}}{2}}({\dot {\psi }}^{2}+{\dot {\phi }}^{2}\cos ^{2}\theta )+I_{3}{\dot {\psi }}{\dot {\phi }}\cos \theta -Mg\ell \cos \theta$

where ψ, φ, θ are the Euler angles, θ is the angle between the vertical z-axis and the top's z′-axis, ψ is the rotation of the top about its own z′-axis, and φ the azimuthal of the top's z′-axis around the vertical z-axis. The principal moments of inertia are I₁ about the top's own x′ axis, I₂ about the top's own y′ axes, and I₃ about the top's own z′-axis. Since the top is symmetric about its z′-axis, I₁ = I₂. Here the simple relation for local gravitational potential energy V = Mglcosθ is used where g is the acceleration due to gravity, and the centre of mass of the top is a distance l from its tip along its z′-axis.

The angles ψ, φ are cyclic. The constant momenta are the angular momenta of the top about its axis and its precession about the vertical, respectively:

$p_{\psi }={\frac {\partial L}{\partial {\dot {\psi }}}}=I_{3}{\dot {\psi }}+I_{3}{\dot {\phi }}\cos \theta$

$p_{\phi }={\frac {\partial L}{\partial {\dot {\phi }}}}={\dot {\phi }}(I_{1}\sin ^{2}\theta +I_{3}\cos ^{2}\theta )+I_{3}{\dot {\psi }}\cos \theta$

From these, eliminating dψ/dt:

$p_{\phi }-p_{\psi }\cos \theta =I_{1}{\dot {\phi }}\sin ^{2}\theta$

we have

${\dot {\phi }}={\frac {p_{\phi }-p_{\psi }\cos \theta }{I_{1}\sin ^{2}\theta }}\,,$

and to eliminate dφ/dt, substitute this result into p_ψ and solve for dψ/dt to find

${\dot {\psi }}={\frac {p_{\psi }}{I_{3}}}-\cos \theta \left({\frac {p_{\phi }-p_{\psi }\cos \theta }{I_{1}\sin ^{2}\theta }}\right)\,.$

The Routhian can be taken to be

$R(\theta ,{\dot {\theta }})=p_{\psi }{\dot {\psi }}+p_{\phi }{\dot {\phi }}-L={\frac {1}{2}}(p_{\psi }{\dot {\psi }}+p_{\phi }{\dot {\phi }})-{\frac {I_{1}{\dot {\theta }}^{2}}{2}}+Mg\ell \cos \theta$

and since

${\frac {p_{\phi }{\dot {\phi }}}{2}}={\frac {p_{\phi }^{2}}{2I_{1}\sin ^{2}\theta }}-{\frac {p_{\psi }p_{\phi }\cos \theta }{2I_{1}\sin ^{2}\theta }}\,,$

${\frac {p_{\psi }{\dot {\psi }}}{2}}={\frac {p_{\psi }^{2}}{2I_{3}}}-{\frac {p_{\psi }p_{\phi }\cos \theta }{2I_{1}\sin ^{2}\theta }}+{\frac {p_{\psi }^{2}\cos ^{2}\theta }{2I_{1}\sin ^{2}\theta }}$

we have

$R={\frac {p_{\psi }^{2}}{2I_{3}}}+{\frac {p_{\psi }^{2}\cos ^{2}\theta }{2I_{1}\sin ^{2}\theta }}+{\frac {p_{\phi }^{2}}{2I_{1}\sin ^{2}\theta }}-{\frac {p_{\psi }p_{\phi }\cos \theta }{4I_{1}\sin ^{2}\theta }}-{\frac {I_{1}{\dot {\theta }}^{2}}{2}}+Mg\ell \cos \theta \,.$

The first term is constant, and can be ignored since only the derivatives of R will enter the equations of motion. The simplified Routhian, without loss of information, is thus

$R={\frac {1}{2I_{1}\sin ^{2}\theta }}\left[p_{\psi }^{2}\cos ^{2}\theta +p_{\phi }^{2}-{\frac {p_{\psi }p_{\phi }}{2}}\cos \theta \right]-{\frac {I_{1}{\dot {\theta }}^{2}}{2}}+Mg\ell \cos \theta$

The equation of motion for θ is, by direct calculation,

${\frac {d}{dt}}{\frac {\partial R}{\partial {\dot {\theta }}}}={\frac {\partial R}{\partial \theta }}\quad \Rightarrow \quad$

$-I_{1}{\ddot {\theta }}=-{\frac {\cos \theta }{I_{1}\sin ^{3}\theta }}\left[p_{\psi }^{2}\cos ^{2}\theta +p_{\phi }^{2}-{\frac {p_{\psi }p_{\phi }}{2}}\cos \theta \right]+{\frac {1}{2I_{1}\sin ^{2}\theta }}\left[-2p_{\psi }^{2}\cos \theta \sin \theta +{\frac {p_{\psi }p_{\phi }}{2}}\sin \theta \right]-Mg\ell \sin \theta \,,$

or by introducing the constants

$a={\frac {p_{\psi }^{2}}{I_{1}^{2}}}\,,\quad b={\frac {p_{\phi }^{2}}{I_{1}^{2}}}\,,\quad c={\frac {p_{\psi }p_{\phi }}{2I_{1}^{2}}}\,,\quad k={\frac {Mg\ell }{I_{1}}}\,,$

a simpler form of the equation is obtained

${\ddot {\theta }}={\frac {\cos \theta }{\sin ^{3}\theta }}(a\cos ^{2}\theta +b-c\cos \theta )+{\frac {1}{2\sin \theta }}(2a\cos \theta -c)+k\sin \theta \,.$

Although the equation is highly nonlinear, there is only one equation to solve for, it was obtained directly, and the cyclic coordinates are not involved.

By contrast, the Lagrangian approach leads to three nonlinear coupled equations to solve, despite the absence of the coordinates ψ and φ in the Lagrangian.

The θ equation is

${\frac {d}{dt}}{\frac {\partial L}{\partial {\dot {\theta }}}}={\frac {\partial L}{\partial \theta }}\quad \Rightarrow \quad I_{1}{\ddot {\theta }}=(I_{1}-I_{3}){\dot {\phi }}^{2}\sin \theta \cos \theta -I_{3}{\dot {\psi }}{\dot {\phi }}\sin \theta +Mg\ell \sin \theta \,,$

the ψ equation is

${\frac {d}{dt}}{\frac {\partial L}{\partial {\dot {\psi }}}}={\frac {\partial L}{\partial \psi }}\quad \Rightarrow \quad {\ddot {\psi }}+{\ddot {\phi }}\cos \theta -{\dot {\phi }}{\dot {\theta }}\sin \theta =0\,,$

and the φ equation is

${\frac {d}{dt}}{\frac {\partial L}{\partial {\dot {\phi }}}}={\frac {\partial L}{\partial \phi }}\quad \Rightarrow \quad {\ddot {\phi }}(I_{1}\sin ^{2}\theta +I_{3}\cos ^{2}\theta )+{\dot {\phi }}(I_{1}-I_{3})2\sin \theta \cos \theta {\dot {\theta }}+I_{3}{\ddot {\psi }}\cos \theta -I_{3}{\dot {\psi }}\sin \theta {\dot {\theta }}=0\,,$

Velocity-dependent potentials

Classical charged particle in a uniform magnetic field

Classical charged particle in uniform B field, using cylindrical coordinates. Top: If the radial coordinate r and angular velocity dθ/dt vary, the trajectory is a helicoid with varying radius but uniform motion in the z direction. Bottom: Constant r and dθ/dt means a helicoid with constant radius.

Consider a classical charged particle of mass m and electric charge q in a static (time-independent) uniform (constant throughout space) magnetic field B. The Lagrangian for a charged particle in a general electromagnetic field given by the magnetic potential A and electric potential φ is

$L={\frac {m}{2}}{\dot {\mathbf {r} }}^{2}-q\phi +q{\dot {\mathbf {r} }}\cdot \mathbf {A} \,,$

It is convenient to use cylindrical coordinates (r, θ, z), so that

${\dot {\mathbf {r} }}=\mathbf {v} =(v_{r},v_{\theta },v_{z})=({\dot {r}},r{\dot {\theta }},{\dot {z}})\,,$

$\mathbf {B} =(B_{r},B_{\theta },B_{z})=(0,0,B)\,.$

In this case the electric potential is zero, φ = 0, and we can choose the axial gauge for the magnetic potential

$\mathbf {A} ={\frac {1}{2}}\mathbf {B} \times \mathbf {r} \quad \Rightarrow \quad \mathbf {A} =(A_{r},A_{\theta },A_{z})=(0,Br/2,0)\,,$

and the Lagrangian is

$L(r,{\dot {r}},{\dot {\theta }},{\dot {z}})={\frac {m}{2}}({\dot {r}}^{2}+r^{2}{\dot {\theta }}^{2}+{\dot {z}}^{2})+{\frac {qBr^{2}{\dot {\theta }}}{2}}\,.$

Notice this potential has an effectively cylindrical symmetry (although it also has angular velocity dependence), since the only spatial dependence is on the radial length from an imaginary cylinder axis.

There are two cyclic coordinates, θ and z. The canonical momenta conjugate to θ and z are the constants

$p_{\theta }={\frac {\partial L}{\partial {\dot {\theta }}}}=mr^{2}{\dot {\theta }}+{\frac {qBr^{2}}{2}}\,,\quad p_{z}={\frac {\partial L}{\partial {\dot {z}}}}=m{\dot {z}}\,,$

so the velocities are

${\dot {\theta }}={\frac {1}{mr^{2}}}\left(p_{\theta }-{\frac {qBr^{2}}{2}}\right)\,,\quad {\dot {z}}={\frac {p_{z}}{m}}\,.$

The angular momentum about the z axis is not p_θ, but the quantity mr²dθ/dt, which is not conserved due to the contribution from the magnetic field. The canonical momentum p_θ is the conserved quantity. It is still the case that p_z is the linear or translational momentum along the z axis, which is also conserved.

The radial component r and angular velocity dθ/dt can vary with time, but p_θ is constant, and since p_z is constant it follows dz/dt is constant. The Routhian can take the form

${\begin{aligned}R(r,{\dot {r}})&=p_{\theta }{\dot {\theta }}+p_{z}{\dot {z}}-L\\&=p_{\theta }{\dot {\theta }}+p_{z}{\dot {z}}-{\frac {m}{2}}{\dot {r}}^{2}-{\frac {p_{\theta }{\dot {\theta }}}{2}}-{\frac {p_{z}{\dot {z}}}{2}}-{\frac {1}{2}}qBr^{2}{\dot {\theta }}\\&=(p_{\theta }-qBr^{2}){\frac {\dot {\theta }}{2}}-{\frac {m}{2}}{\dot {r}}^{2}+{\frac {p_{z}{\dot {z}}}{2}}\\&={\frac {1}{2mr^{2}}}\left(p_{\theta }-qBr^{2}\right)\left(p_{\theta }-{\frac {qBr^{2}}{2}}\right)-{\frac {m}{2}}{\dot {r}}^{2}+{\frac {p_{z}^{2}}{2m}}\\&={\frac {1}{2mr^{2}}}\left(p_{\theta }^{2}-{\frac {3}{2}}qBr^{2}+{\frac {(qB)^{2}r^{4}}{2}}\right)-{\frac {m}{2}}{\dot {r}}^{2}\end{aligned}}$

where in the last line, the p_z²/2m term is a constant and can be ignored without loss of continuity. The Hamiltonian equations for θ and z automatically vanish and do not need to be solved for. The Lagrangian equation in r

${\frac {d}{dt}}{\frac {\partial R}{\partial {\dot {r}}}}={\frac {\partial R}{\partial r}}$

is by direct calculation

$-m{\ddot {r}}={\frac {1}{2m}}\left[{\frac {-2}{r^{3}}}\left(p_{\theta }^{2}-{\frac {3}{2}}qBr^{2}+{\frac {(qB)^{2}r^{4}}{2}}\right)+{\frac {1}{r^{2}}}(-3qBr+2(qB)^{2}r^{3})\right]\,,$

which after collecting terms is

$m{\ddot {r}}={\frac {1}{2m}}\left[{\frac {2p_{\theta }^{2}}{r^{3}}}-(qB)^{2}r\right]\,,$

and simplifying further by introducing the constants

$a={\frac {p_{\theta }^{2}}{m^{2}}}\,,\quad b=-{\frac {(qB)^{2}}{2m^{2}}}\,,$

the differential equation is

${\ddot {r}}={\frac {a}{r^{3}}}+br$

To see how z changes with time, integrate the momenta expression for p_z above

$z={\frac {p_{z}}{m}}t+c_{z}\,,$

where c_z is an arbitrary constant, the initial value of z to be specified in the initial conditions.

The motion of the particle in this system is helicoidal, with the axial motion uniform (constant) but the radial and angular components varying in a spiral according to the equation of motion derived above. The initial conditions on r, dr/dt, θ, dθ/dt, will determine if the trajectory of the particle has a constant r or varying r. If initially r is nonzero but dr/dt = 0, while θ and dθ/dt are arbitrary, then the initial velocity of the particle has no radial component, r is constant, so the motion will be in a perfect helix. If r is constant, the angular velocity is also constant according to the conserved p_θ.

With the Lagrangian approach, the equation for r would include dθ/dt which has to be eliminated, and there would be equations for θ and z to solve for.

The r equation is

${\frac {d}{dt}}{\frac {\partial L}{\partial {\dot {r}}}}={\frac {\partial L}{\partial r}}\quad \Rightarrow \quad m{\ddot {r}}=mr{\dot {\theta }}^{2}+qBr{\dot {\theta }}\,,$

the θ equation is

${\frac {d}{dt}}{\frac {\partial L}{\partial {\dot {\theta }}}}={\frac {\partial L}{\partial \theta }}\quad \Rightarrow \quad m(2r{\dot {r}}{\dot {\theta }}+r^{2}{\ddot {\theta }})+qBr{\dot {r}}=0\,,$

and the z equation is

${\frac {d}{dt}}{\frac {\partial L}{\partial {\dot {z}}}}={\frac {\partial L}{\partial z}}\quad \Rightarrow \quad m{\ddot {z}}=0\,.$

The z equation is trivial to integrate, but the r and θ equations are not, in any case the time derivatives are mixed in all the equations and must be eliminated.

See also

• Phase space
• Configuration space
• Many-body problem
• Rigid body mechanics

References

• Landau, L. D.; Lifshitz, E. M. Mechanics (3rd ed.). Butterworth Heinemann. p. 134. ISBN 9780750628969.
• Hand, L. N.; Finch, J. D. Analytical Mechanics (2nd ed.). Cambridge University Press. p. 23. ISBN 9780521575720.
• Kibble, T. W. B.; Berkshire, F. H. (2004). Classical Mechanics (5th ed.). Imperial College Press. p. 236. ISBN 9781860944352.
• Goldstein, Herbert (1980). Classical Mechanics (2nd ed.). San Francisco, CA: Addison Wesley. pp. 352–353. ISBN 0201029189.
• Goldstein, Herbert; Poole, Charles P., Jr.; Safko, John L. (2002). Classical Mechanics (3rd ed.). San Francisco, CA: Addison Wesley. pp. 347–349. ISBN 0-201-65702-3.{{cite book}}: CS1 maint: multiple names: authors list (link)