Chandrasekhar–Kendall function

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

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

where $\hat{\mathbf{n}}$ 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., $\mathrm{\nabla }\times \mathbf{v}=\lambda \mathbf{v}$.

Derivation

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

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

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

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

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

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

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

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

Cylindrical polar coordinates

Taking the unit vector in the $z$ direction, i.e., $\hat{\mathbf{n}}={\mathbf{e}}_z$, 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, $$\begin{gathered} k=\pm 2\pi n/L, \\ n=0,1,2,\dots \end{gathered}$$, 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 $\hat{\mathbf{n}}={\mathbf{e}}_z$, 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