Chandrasekhar–Kendall function

Template:Short description Chandrasekhar–Kendall functions are the eigenfunctions of the curl operator derived by Subrahmanyan Chandrasekhar and P. C. Kendall in 1957 while attempting to solve the force-free magnetic fields. The functions were independently derived by both, and the two decided to publish their findings in the same paper.

If the force-free magnetic field equation is written as $\mathrm{\nabla }\times 𝐇=\lambda 𝐇$, where $𝐇$ is the magnetic field and $\lambda$ is the force-free parameter, with the assumption of divergence free field, $\mathrm{\nabla }\cdot 𝐇=0$, then the most general solution for the axisymmetric case is

$𝐇=\frac{1}{\lambda }\mathrm{\nabla }\times (\mathrm{\nabla }\times \psi \widehat{𝐧})+\mathrm{\nabla }\times \psi \widehat{𝐧}$

where $\widehat{𝐧}$ is a unit vector and the scalar function $\psi$ satisfies the Helmholtz equation, i.e.,

${\mathrm{\nabla }}^2\psi +{\lambda }^2\psi =0.$

The same equation also appears in Beltrami flows from fluid dynamics where, the vorticity vector is parallel to the velocity vector, i.e., $\mathrm{\nabla }\times 𝐯=\lambda 𝐯$.

Derivation

Taking curl of the equation $\mathrm{\nabla }\times 𝐇=\lambda 𝐇$ and using this same equation, we get

$\mathrm{\nabla }\times (\mathrm{\nabla }\times 𝐇)={\lambda }^2𝐇$.

In the vector identity $\mathrm{\nabla }\times (\mathrm{\nabla }\times 𝐇)=\mathrm{\nabla }(\mathrm{\nabla }\cdot 𝐇)-{\mathrm{\nabla }}^2𝐇$, we can set $\mathrm{\nabla }\cdot 𝐇=0$ since it is solenoidal, which leads to a vector Helmholtz equation,

${\mathrm{\nabla }}^2𝐇+{\lambda }^2𝐇=0$.

Every solution of above equation is not the solution of original equation, but the converse is true. If $\psi$ is a scalar function which satisfies the equation ${\mathrm{\nabla }}^2\psi +{\lambda }^2\psi =0$, then the three linearly independent solutions of the vector Helmholtz equation are given by

$𝐋=\mathrm{\nabla }\psi ,𝐓=\mathrm{\nabla }\times \psi \widehat{𝐧},𝐒=\frac{1}{\lambda }\mathrm{\nabla }\times 𝐓$

where $\widehat{𝐧}$ is a fixed unit vector. Since $\mathrm{\nabla }\times 𝐒=\lambda 𝐓$, it can be found that $\mathrm{\nabla }\times (𝐒+𝐓)=\lambda (𝐒+𝐓)$. But this is same as the original equation, therefore $𝐇=𝐒+𝐓$, where $𝐒$ is the poloidal field and $𝐓$ is the toroidal field. Thus, substituting $𝐓$ in $𝐒$, we get the most general solution as

$𝐇=\frac{1}{\lambda }\mathrm{\nabla }\times (\mathrm{\nabla }\times \psi \widehat{𝐧})+\mathrm{\nabla }\times \psi \widehat{𝐧}.$

Cylindrical polar coordinates

Taking the unit vector in the $z$ direction, i.e., $\widehat{𝐧}={𝐞}_z$, with a periodicity $L$ in the $z$ direction with vanishing boundary conditions at $r=a$, the solution is given by

$\psi =J_m({\mu }_{j}r)e^{im\theta +ikz},\lambda =\pm ({\mu }_j^2+k^2{)}^{1/2}$

where $J_m$ is the Bessel function, $k=\pm 2\pi n/L,n=0,1,2,\dots$, the integers $m=0,\pm 1,\pm 2,\dots$ and ${\mu }_j$ is determined by the boundary condition $ak{\mu }_j{J_m}^{\prime }({\mu }_{j}a)+m\lambda J_m({\mu }_{j}a)=0.$ The eigenvalues for $m=n=0$ has to be dealt separately. Since here $\widehat{𝐧}={𝐞}_z$, we can think of $z$ direction to be toroidal and $\theta$ direction to be poloidal, consistent with the convention.

See also

• Poloidal–toroidal decomposition
• Woltjer's theorem