---
author:
- 'M. Gellert'
- 'G. Rüdiger'
- 'D. Elstner'
title: 'Helicity generation and $\alpha$-effect by Tayler instability with $z$-dependent differential rotation'
---

Introduction
============

Helicity in rotating turbulence plays a basic role in dynamo theory for the generation of large-scale cosmic magnetic fields [@krause_1980; @brandenb_2005]. Usually stratification of density or turbulence itself is needed to generate helicity. We demonstrate that, even without stratification, helicity can exist due to the common action of magnetic fields and differential rotation. Whereas differential rotation depending on latitude is well-known from observations of star spots, differential rotation (of the interior of stars) depending on the $z$-coordinate only, appears more rarely. It is predicted and observable, for instance, in the tachocline of the sun (Rüdiger & Kitchatinov 1997; Kitchatinov & Rüdiger 2005), and influences the internal rotation of massive stars [@maeder]. It may open the possibility of studying nonaxisymmetric (large-scale) structures by shear-driven magnetohydrodynamic (MHD) instability of laminar flows [@braithspruit_2004; @braithw_2006].\
Differential rotation transforms poloidal field components into toroidal components, which due to the Tayler instability (TI), become unstable if a critical amplitude is exceeded (Vandakurov 1972). Tayler (1973) showed that a magnetic field $B_{\phi}$ becomes unstable against nonaxisymmetric perturbations if the condition $$\frac{\mathrm{d}}{\mathrm{d} R} \left(R B_{\phi}^2\right) < 0,$$ where cylindrical coordinates $(R,\phi,z)$ are used, is violated. Constant fields or fields $B_{\phi}\propto R$, like those produced by $z$-dependent differential rotation from an axial field, are candidates for this instability. The most unstable Fourier mode for such a configuration is the nonaxisymmetric mode $m=1$ despite the smoothing action of the differential rotation. In a mean-field approach, due to the relation $$\label{alpha}
\alpha \simeq - \frac{\tau_{\rm corr}}{3}{\cal H},$$ helicity ${\cal H}= {\cal H}_{\rm kin}- {\cal H}_{\rm curr}$ often indicates an existing $\alpha$-effect. ${\cal H}_{\rm kin}$ and ${\cal H}_{\rm curr}$ are the kinematic and current helicity, $$\label{heli}
{\cal H}_{\rm kin} =\langle\vec{u}' \cdot {\rm rot}\, \vec{u}'\rangle, \quad {\cal H}_{\rm curr}= \frac{1}{\mu_0 \rho} \langle \vec{B}'\cdot {\rm rot}\vec{B}'\rangle,$$ respectively and $\tau_{\rm corr}$ is the correlation time of the field pattern. Nonvanishing helicity could indeed be an indication of the existence of a resulting $\alpha$-effect on the basis of the TI. In case of the presence of an external field $\f{B}^0$ and with a large magnetic Reynolds number, a dominating contribution from magnetic-field fluctuations to the $\alpha$-effect can arise (Pouquet, Frisch & Leorat 1976; Brandenburg & Subramanian 2007).\
Keeping in mind the pseudoscalar nature of helicity, a possible relation between helicity and both the external field and differential rotation would be $$\label{h1}
{\cal H} \propto B^0_i\, B^0_j\, {{\it \Omega}}_{i,j},$$ where $B^0_i$ means the external field components and ${{\it \Omega}}_{i,j}$ the gradient tensor of the basic rotation. The sign of ${\cal H}$ in Eq. (\[h1\]) does not depend on the sign of the magnetic field, but it depends on the sign of the shear ${{\it \Omega}}_{i,j}$. Consequently, the dynamo number $$D = \frac{L^2\, \alpha\, {{\it \Omega}}}{\eta_{\rm T}^2},$$ would now have a positive-definite sign. Here $L$ is the characteristic scale of the cylinder domain and $\eta_{\rm T}\simeq \tau_{\rm corr} \langle{u'}^2\rangle$. The sign of the dynamo number determines important properties of possible dynamo processes. E.g., a simple disk dynamo oscillates for a positive dynamo number and it is stationary for a negative dynamo number. Also, the magnetic Reynolds number of the $\alpha$-effect itself is important, that is, with Eq. (\[alpha\]) including the magnetic contribution, $$C_\alpha= \frac{L |\cal{H}|}{\langle u'^2\rangle}
\label{Caa}$$ ($\eta_{\rm T}$ does not include magnetic contributions, Vainshtein & Kitchatinov 1983). We shall see that after the onset of TI, this quantity is of the order of unity when the averages are taken as an integral over the azimuthal direction.

In the following, the details of the model used are explained. Section \[sec\_instability\] describes the onset of the TI in a cylindrical enclosure and the resulting field structure. In Sect. \[sec\_helicity\], it is shown that – if the axial field is strong enough – the numerical simulations are in good agreement with relation \[h1\] in the case of $z$-dependent differential rotation, where it simplifies to ${\cal H} \propto {B^0_z}^2 \mathrm{d}{{\it \Omega}}/\mathrm{d}z$ and only a (strong enough) $z$-component $B^0_z$ of the external field is needed. In Sect. \[sec\_alpha\] we show that the generated helicity is connected with an $\alpha$-effect, which is also proportional to the gradient of the differential rotation.

Model
=====

We consider a differentially-rotating cylinder with radius $L$ and height $L$ embedded in a box with cartesian grid of side length $2.5L$ and height $L$ (see Fig. \[fig\_sketch\_cyl\]). The cylinder radius is 20% less than the box side length, which appeared to be a good compromise between wasted computing power in the corner regions and decreasing influence from the geometry of the box. We calculated using the PENCIL code [@brandenb_2002], a high-order finite difference code (sixth order in space and third order in time). Inside the cylinder domain, we solve both momentum and induction equations. Outside the cylinder, we kept the initial velocity to sustain the differential rotation via this no-slip conditions on the rim of the cylinder. On the top and the bottom, we apply stress-free conditions for the flow.

For the magnetic field, perfect conductor boundary conditions are applied on all box boundaries. Additionally, in the region outside the cylinder, magnetic diffusivity $\eta$ is enhanced to a value ten times larger than inside the cylinder.\
To keep the system nearly incompressible with a code for compressible media, the value of ${{\it \Omega}}(z)$ is chosen in a way that the resulting maximum of the (meridional) velocity never exceeds 16% of the speed of sound, which was set to $c_{\rm s}=8$. The initial density is set to $\varrho_0=1$, fluctuations are of the order of $10^{-4}$. The spatial resolution is $N=96\times$96$\times$48. Test runs with $N=128\times$128$\times$96 deliver only slight differences with smoother fields.\
The initial magnetic field consists of the external time-independent homogeneous field $\f{B}^0=(0,0,B^0_z)$ applied only inside the cylinder. It is twisted into a strong toroidal field by the differential rotation. The strength of the generated field depends on $B^0_z$, varied between $B^0_z=0.01$ and $B^0_z=0.1$, and the gradient of the differential rotation $\mathrm{d}{{\it \Omega}}/\mathrm{d}z$, where the latter was fixed to $|\mathrm{d}{{\it \Omega}}/\mathrm{d}z| = 1$ for all presented calculations. Based on the radius (set to $L = 1$) and the velocity at $z=1$ ($U={{\it \Omega}}L=1$), and the viscosity ($\nu=0.03$), the Reynolds number has a value of $\mathrm{Re}=33$. In the following text, system rotation always refers to the rotation on top of the cylinder and time is given in units of rotation time. The magnetic Prandtl number $\mathrm{Pm}$ is varied between $\mathrm{Pm}=10$ and $\mathrm{Pm}=30$ with no qualitatively change of the instability. In the following analysis, we concentrate on $\mathrm{Pm}=15$. We choose a large Prandtl number to encourage dynamo action, although we observed no dynamo.

Instability {#sec_instability}
===========

If $B_{\phi}$ becomes strong enough, the TI occurs and leads to a growing nonaxisymmetric field. The largest nonaxisymmetric mode is $m=1$. By “strong enough" we mean that not only does the magnitude of $B_{\phi}$ reach high enough values, but also a certain threshold $B_{\phi}/B^0_z$ (with $B_{\phi}/B^0_z$ of the order of $\mathrm{Pm}$) needs to be crossed, which is different from the case of pure toroidal fields (Tayler 1973; see Rüdiger et al. 2007). This means that an additional poloidal field component suppresses the instability. For $\mathrm{Pm}=15$, the instability sets in at a Hartmann number of $\mathrm{Ha}=B^{\ast} R/\sqrt{\mu_0 \varrho \nu \eta}=130$, where $B^{\ast}\approx 1$ means the maximal value of the generated toroidal field $B_{\phi}$. To produce such a strong toroidal component an external field $B^0_z \ge 0.04$ is needed. The instability did not occur for $B^0_z > 0.08$.\
The nonaxisymmetric structures appear first near the axis in the lower part of the cylinder where velocity magnitude is small, and grows to the steady state (Fig. \[fig\_bpower\]). For $B_R$ and $B_z$, the $m=1$ mode becomes the largest one, in $B_{\phi}$ the axisymmetric mode remains dominant due to the permanently reproduced axisymmetric field. In the nonlinear regime, before the steady state is reached, higher modes also appear. Nonetheless, their magnitudes stay below 10% of the $m=1$ mode. One exception is the $m=4$ mode, caused by the box geometry. During the initial phase, this mode is already present and influences the magnetic field outside the cylinder near the box boundaries. However, the field inside the cylinder is much less affected, and the $m=4$ mode does not seem to influence the nature and onset of the instability at all. Additionally, during the growth phase of all other nonaxisymmetric modes, the $m=4$ remains nearly unchanged and does not play an extraordinary role in the final state. Modes higher than $m=4$ are not plotted in Fig. \[fig\_bpower\].

The pattern of the $m=1$ mode (Fig. \[fig\_m1\]) possesses an azimuthal drift velocity relative to the system rotation. It rotates with $4.5$ rotation periods of the cylinder, independent of the strength of the externally applied field. The TI in a Taylor-Couette system exhibits the same characteristics of the unstable mode [@rued_destab].

Generation of helicity {#sec_helicity}
======================

To test the relation described by Eq. (\[h1\]) in a simple setup, we restricted differential rotation to depend only on the $z$-direction. [^1] For this case, the helicity ${\cal H}$ should depend on the sign of $\mathrm{d}{{\it \Omega}}/\mathrm{d}z$, but not on the sign of the external field and scale with the squared value of the latter, i.e. ${\cal H} \propto {B^0_z}^2\, \mathrm{d}{{\it \Omega}}/\mathrm{d}z$. During the onset of the instability, the deviation of the flow structure from the original toroidal field is comparable to that of the magnetic field. Also, here the mode $m=1$ is the largest nonaxisymmetric mode and the higher modes appear with less energy.\
For the definition of fluctuations, we average velocity and magnetic field along the azimuthal direction, i.e. $$\langle \f{u}\rangle = \frac{1}{2\pi} \oint \f{u}\, \mathrm{d}\phi, \quad \langle \f{B}\rangle = \frac{1}{2\pi} \oint \f{B}\, \mathrm{d}\phi,$$ and regard the nonaxisymmetric parts as fluctuations of the fields. For constant $\mathrm{d}{{\it \Omega}}/\mathrm{d}z$, and with a homogeneous external field, the fluctuations should be constant in the vertical direction. Due to the finite height of the cylinder, boundary effects near the top and bottom induce additional flow disturbances and changes in the structure of the magnetic field in these regions. The independence is roughly preserved in the central region between $z=0.35$ and $z=0.65$. In Fig. \[fig\_marc4\] we show the energies of the fluctuations of velocity and magnetic field averaged over this central region, and their dependence on the external field $B^0_z$. The values are taken in radial direction at $R=0.5$. The magnetic energy always exceeds the kinetic energy. The ratio varies between $15$ and $30$. Thus, the instability is dominated by the magnetic field. This is also reflected in the helicities. We again use azimuthal-averaged quantities, $${\cal H}_{\rm kin}\!=\! \frac{1}{2\pi}\! \oint \f{u}' \cdot {\rm rot}\,\f{u}' \, \mathrm{d}\phi, \quad 
 {\cal H}_{\rm curr}\! =\! \frac{1}{2\pi\mu_0\rho}\! \oint \f{B}' \cdot {\rm rot}\,\f{B}'\, \mathrm{d}\phi.$$ Both are zero as long as no instability exists, with proceeding instability and growing nonaxisymmetric modes the helicity quantities also become unequal to zero. An example plot of ${\cal H}_{\rm kin}$ for $R=0.5$ and $z=0.5$ is shown in Fig. \[fig\_hk\_hc\].

After a transition, a steady-state value is reached for both ${\cal H}_{\rm kin}$ and ${\cal H}_{\rm curr}$. The current helicity is approximately 40 times larger than the kinetic helicity in the example shown in the center of the cylinder. In the vertical direction we observed the same behavior as for the fluctuations of flow and magnetic field. Near the top and bottom, the helicities are stronger than those in the region between $z=0.35$ and $z=0.65$. For a positive gradient in angular velocity ${\cal H}_{\rm kin}$ is negative and ${\cal H}_{\rm curr}$ positive. With the changing sign of $\mathrm{d}\Omega/\mathrm{d}z$, the sign of ${\cal H}_{\rm kin}$ and ${\cal H}_{\rm curr}$ also changes, whereas the sign of $B^0_z$ has no influence. And, as expected, the absolute value of ${\cal H}_{\rm kin}$ is proportional to the squared value of the external field. For $\mathrm{Pm}=15$ the relation between $B^0_z$ and ${\cal H}_{\rm kin}$ is shown in Fig. \[fig\_hk\_b02\]. The fitted parabola does not exactly cross the origin. This shift is attributed to the instability requiring a certain value of $B^0_z$ (i.e. $B^0_z=0.04$ for $\mathrm{Pm}=15$) to set in with a certain value for ${\cal H}_{\rm kin}$ larger than zero.

Alpha effect {#sec_alpha}
============

Equation (\[alpha\]) suggests that the changing sign of the helicities by changing the direction of $\mathrm{d}{{\it \Omega}}/\mathrm{d}z$ will also appear for the term $\alpha_{zz}$ in the $\alpha$-tensor responsible for the regeneration of the magnetic field. Indeed, calculating $\alpha_{zz}={ \langle\f{u}' \times \f{B}'\rangle}_z/B^0_z$ using the $z$-component of the electromotive force, gives values for $\alpha_{zz}$ with the same sign as $\mathrm{d}{{\it \Omega}}/\mathrm{d}z$ for $z<0.65$ (see Fig. \[fig\_alpha\]). Near the top boundary, the disturbances already discussed for the helicities change the values of $\alpha_{zz}$ dramatically to the opposite sign. We excluded this region and took mean values of $\alpha_{zz}$ in the same range $0.35<z<0.65$ used for the helicities and find coefficients between $\alpha_{zz} = 0.038$ for $B^0_z=0.04$ and $\alpha_{zz} = 0.067$ for $B^0_z=0.08$. The correlation time derived from expression (\[alpha\]) using both helicities, $\tau_{\rm corr} = 3 \alpha_{zz} / ({\cal H}_{\rm curr} - {\cal H}_{\rm kin})$, is of the order of the system rotation time. Note that the $\alpha$-effect here is mainly due to the current helicity and the product $\alpha_{zz}{\cal H}_{\rm curr}$ is positive.

If the external field is switched off, all magnetic field modes decay in the investigated parameter region of low Reynolds numbers and magnetic Prandtl numbers of the order of ten. The helicities drop down to zero nearly immediately. Despite the high magnetic Prandtl number, we do not observe any dynamo action, as found in comparable geometry [@braithw_2006]. Also, the reported cyclic behavior of the instability did not occur in our simulations.

Conclusions
===========

We have demonstrated how the instability of toroidal magnetic fields leads to helicity generation in the nonaxisymmetric parts of a flow without density stratification. The suggested relation between helicity, external field, and differential rotation, ${\cal H} \propto B^0_i\, B^0_j\, {{\it \Omega}}_{i,j}$, is rather well fulfilled in the case of $z$-dependent differential rotation. Both the kinematic helicity and current helicity depend on the squared value of the $z$-component of the external magnetic field $B^0_z$, and scale linearly with the gradient of the differential rotation. Also, the magnetically dominated $\alpha$-effect depends on the direction of $\mathrm{d}{{\it \Omega}}/\mathrm{d}z$, that is $\alpha_{zz}$ holds the same sign as $\mathrm{d}{{\it \Omega}}/\mathrm{d}z$.\
The realized model is too simple to estimate consequences of an $\alpha$-effect based on this new kind of helicity production for environments without density stratification and possibly for new dynamo models. In a next step, therefore, we would like to check the relation (\[h1\]) when differential rotation depending on the distance from the rotation axis is present as well. With an appropriate flow it becomes ${\cal H}_{\rm kin} \propto B^0_R B^0_z \mathrm{d}{{\it \Omega}}/\mathrm{d}R$. In this case, helicity generation should be observable only if both components of the external field are unequal to zero. The problem with this constellation is the changing sign of the product of both field components in one hemisphere in the simplest configuration, a dipole-like field.

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[^1]: The resulting non-conservative centrifugal force drives a meridional flow that, however, remains small (see Fig. \[fig\_bpower\]).
