Digital Library of Mathematical Functions
About the Project
NIST
22 Jacobian Elliptic FunctionsApplications

§22.19 Physical Applications

Show Annotations
Referenced by:
§22.1
Permalink:
http://dlmf.nist.gov/22.19
Contents

§22.19(i) Classical Dynamics: The Pendulum

Show Annotations
Notes:
See Lawden (1989, pp. 114–117). Figure 22.19.1 was produced at NIST.
Keywords:
Jacobian elliptic functions, amplitude (\mathop{\mathrm{am}\/}\nolimits) function, pendulum
Permalink:
http://dlmf.nist.gov/22.19.i

With appropriate scalings, Newton’s equation of motion for a pendulum with a mass in a gravitational field constrained to move in a vertical plane at a fixed distance from a fulcrum is

\theta being the angular displacement from the point of stable equilibrium, \theta=0. The bounded (-\pi\leq\theta\leq\pi) oscillatory solution of (22.19.1) is traditionally written

for an initial angular displacement \alpha, with \ifrac{d\theta}{dt}=0 at time 0; see Lawden (1989, pp. 114–117). The period is 4\!\mathop{K\/}\nolimits\!\left(\mathop{\sin\/}\nolimits\!\left(\frac{1}{2}% \alpha\right)\right). The angle \alpha=\pi is a separatrix, separating oscillatory and unbounded motion. With the same initial conditions, if the sign of gravity is reversed then the new period is 4\!\mathop{{K^{{\prime}}}\/}\nolimits\!\left(\mathop{\sin\/}\nolimits\!\left(% \frac{1}{2}\alpha\right)\right); see Whittaker (1964, §44).

Alternatively, Sala (1989) writes:

for the initial conditions \theta(0)=0, the point of stable equilibrium for E=0, and \ifrac{d\theta(t)}{dt}=\sqrt{2E}. Here E=\frac{1}{2}(\ifrac{d\theta(t)}{dt})^{2}+1-\mathop{\cos\/}\nolimits\theta(t) is the energy, which is a first integral of the motion. This formulation gives the bounded and unbounded solutions from the same formula (22.19.3), for k\geq 1 and k\leq 1, respectively. Also, \theta(t) is not restricted to the principal range -\pi\leq\theta\leq\pi. Figure 22.19.1 shows the nature of the solutions \theta(t) of (22.19.3) by graphing \mathop{\mathrm{am}\/}\nolimits\left(x,k\right) for both 0\leq k\leq 1, as in Figure 22.16.1, and k\geq 1, where it is periodic.

See accompanying text
Figure 22.19.1: Jacobi’s amplitude function \mathop{\mathrm{am}\/}\nolimits\left(x,k\right) for 0\leq x\leq 10\pi and k=0.5,0.9999,1.0001,2. When k<1, \mathop{\mathrm{am}\/}\nolimits\left(x,k\right) increases monotonically indicating that the motion of the pendulum is unbounded in \theta, corresponding to free rotation about the fulcrum; compare Figure 22.16.1. As k\to 1-, plateaus are seen as the motion approaches the separatrix where \theta=n\pi, n=\pm 1,\pm 2,..., at which points the motion is time independent for k=1. This corresponds to the pendulum being “upside down” at a point of unstable equilibrium. For k>1, the motion is periodic in x, corresponding to bounded oscillatory motion. Magnify

§22.19(ii) Classical Dynamics: The Quartic Oscillator

Show Annotations
Notes:
See Lawden (1989, pp. 117–119).
Keywords:
Jacobian elliptic functions, quartic oscillator
Referenced by:
§23.21(i)
Permalink:
http://dlmf.nist.gov/22.19.ii

Classical motion in one dimension is described by Newton’s equation

where V(x) is the potential energy, and x(t) is the coordinate as a function of time t. The potential

plays a prototypal role in classical mechanics (Lawden (1989, §5.2)), quantum mechanics (Schulman (1981, Chapter 29)), and quantum field theory (Pokorski (1987, p. 203), Parisi (1988, §14.6)). Its dynamics for purely imaginary time is connected to the theory of instantons (Itzykson and Zuber (1980, p. 572), Schäfer and Shuryak (1998)), to WKB theory, and to large-order perturbation theory (Bender and Wu (1973), Simon (1982)).

For \beta real and positive, three of the four possible combinations of signs give rise to bounded oscillatory motions. We consider the case of a particle of mass 1, initially held at rest at displacement a from the origin and then released at time t=0. The subsequent position as a function of time, x(t), for the three cases is given with results expressed in terms of a and the dimensionless parameter \eta=\frac{1}{2}\beta a^{2}.

Case I: V(x)=\frac{1}{2}x^{2}+\frac{1}{4}\beta x^{4}

This is an example of Duffing’s equation; see Ablowitz and Clarkson (1991, pp. 150–152) and Lawden (1989, pp. 117–119). The subsequent time evolution is always oscillatory with period 4\!\mathop{K\/}\nolimits\!\left(k\right)/\sqrt{1+\eta}:

Case II: V(x)=\frac{1}{2}x^{2}-\frac{1}{4}\beta x^{4}

There is bounded oscillatory motion near x=0, with period 4\!\mathop{K\/}\nolimits\!\left(k\right)/\sqrt{1-\eta}, for initial displacements with |a|\leq\sqrt{1/\beta}:

As a\to\sqrt{1/\beta} from below the period diverges since a=\pm\sqrt{1/\beta} are points of unstable equilibrium.

Case III: V(x)=-\frac{1}{2}x^{2}+\frac{1}{4}\beta x^{4}

Two types of oscillatory motion are possible. For an initial displacement with \sqrt{1/\beta}\leq|a|\leq\sqrt{2/\beta}, bounded oscillations take place near one of the two points of stable equilibrium x=\pm\sqrt{1/\beta}. Such oscillations, of period 4\!\mathop{K\/}\nolimits\!\left(k\right)/\sqrt{\eta}, are given by:

As a\to\sqrt{2/\beta} from below the period diverges since x=0 is a point of unstable equlilibrium. For initial displacement with |a|\geq\sqrt{2/\beta} the motion extends over the full range -a\leq x\leq a:

with period 4\!\mathop{K\/}\nolimits\!\left(k\right)/\sqrt{2\eta-1}. As |a|\to\sqrt{2/\beta} from above the period again diverges. Both the \mathop{\mathrm{dn}\/}\nolimits and \mathop{\mathrm{cn}\/}\nolimits solutions approach a\mathop{\mathrm{sech}\/}\nolimits t as a\to\sqrt{2/\beta} from the appropriate directions.

§22.19(iii) Nonlinear ODEs and PDEs

Many nonlinear ordinary and partial differential equations have solutions that may be expressed in terms of Jacobian elliptic functions. These include the time dependent, and time independent, nonlinear Schrödinger equations (NLSE) (Drazin and Johnson (1993, Chapter 2), Ablowitz and Clarkson (1991, pp. 42, 99)), the Korteweg–de Vries (KdV) equation (Kruskal (1974), Li and Olver (2000)), the sine-Gordon equation, and others; see Drazin and Johnson (1993, Chapter 2) for an overview. Such solutions include standing or stationary waves, periodic cnoidal waves, and single and multi-solitons occurring in diverse physical situations such as water waves, optical pulses, quantum fluids, and electrical impulses (Hasegawa (1989), Carr et al. (2000), Kivshar and Luther-Davies (1998), and Boyd (1998, Appendix D2.2)).

§22.19(iv) Tops

The classical rotation of rigid bodies in free space or about a fixed point may be described in terms of elliptic, or hyperelliptic, functions if the motion is integrable (Audin (1999, Chapter 1)). Hyperelliptic functions u(z) are solutions of the equation z=\int_{0}^{u}(f(x))^{{-1/2}}dx, where f(x) is a polynomial of degree higher than 4. Elementary discussions of this topic appear in Lawden (1989, §5.7), Greenhill (1959, pp. 101–103), and Whittaker (1964, Chapter VI). A more abstract overview is Audin (1999, Chapters III and IV), and a complete discussion of analytical solutions in the elliptic and hyperelliptic cases appears in Golubev (1960, Chapters V and VII), the original hyperelliptic investigation being due to Kowalevski (1889).

§22.19(v) Other Applications

Numerous other physical or engineering applications involving Jacobian elliptic functions, and their inverses, to problems of classical dynamics, electrostatics, and hydrodynamics appear in Bowman (1953, Chapters VII and VIII) and Lawden (1989, Chapter 5). Whittaker (1964, Chapter IV) enumerates the complete class of one-body classical mechanical problems that are solvable this way.

© 2010–2013 NIST / Privacy Policy / Disclaimer / Feedback; Version 1.0.6; Release date 2013-05-06 Math-Image version (See MathML) . A Printed Companionis available.