Stokes stream function

In fluid dynamics, the Stokes stream function is used to describe the streamlines and flow velocity in a three-dimensional incompressible flow with axisymmetry. A surface with a constant value of the Stokes stream function encloses a streamtube, everywhere tangential to the flow velocity vectors. Further, the volume flux within this streamtube is constant, and all the streamlines of the flow are located on this surface. The velocity field associated with the Stokes stream function is solenoidal—it has zero divergence. This stream function is named in honor of George Gabriel Stokes.

Streamlines around a sphere in axisymmetric Stokes flow. At terminal velocity the drag force F_d balances the force F_g propelling the object.

Cylindrical coordinates

A point plotted with cylindrical coordinates.

Consider a cylindrical coordinate system ( ρ , φ , z ), with the z–axis the line around which the incompressible flow is axisymmetrical, φ the azimuthal angle and ρ the distance to the z–axis. Then the flow velocity components u_ρ and u_z can be expressed in terms of the Stokes stream function $\Psi$ by:[1]

{\begin{aligned}u_{\rho }&=-{\frac {1}{\rho }}\,{\frac {\partial \Psi }{\partial z}},\\u_{z}&=+{\frac {1}{\rho }}\,{\frac {\partial \Psi }{\partial \rho }}.\end{aligned}}

The azimuthal velocity component u_φ does not depend on the stream function. Due to the axisymmetry, all three velocity components ( u_ρ , u_φ , u_z ) only depend on ρ and z and not on the azimuth φ.

The volume flux, through the surface bounded by a constant value ψ of the Stokes stream function, is equal to 2π ψ.

Spherical coordinates

A point plotted using the spherical coordinate system

In spherical coordinates ( r , θ , φ ), r is the radial distance from the origin, θ is the zenith angle and φ is the azimuthal angle. In axisymmetric flow, with θ = 0 the rotational symmetry axis, the quantities describing the flow are again independent of the azimuth φ. The flow velocity components u_r and u_θ are related to the Stokes stream function $\Psi$ through:[2]

{\begin{aligned}u_{r}&=+{\frac {1}{r^{2}\,\sin \theta }}\,{\frac {\partial \Psi }{\partial \theta }},\\u_{\theta }&=-{\frac {1}{r\,\sin \theta }}\,{\frac {\partial \Psi }{\partial r}}.\end{aligned}}

Again, the azimuthal velocity component u_φ is not a function of the Stokes stream function ψ. The volume flux through a stream tube, bounded by a surface of constant ψ, equals 2π ψ, as before.

Vorticity

The vorticity is defined as:

{\boldsymbol {\omega }}=\nabla \times {\boldsymbol {u}}=\nabla \times \nabla \times {\boldsymbol {\psi }}

, where

{\boldsymbol {\psi }}=-{\frac {\Psi }{r\sin \theta }}{\boldsymbol {\hat {\phi }}},

with ${\boldsymbol {\hat {\phi }}}$ the unit vector in the $\phi \,$ –direction.

Derivation of vorticity

{\boldsymbol {\omega }}

using a Stokes stream function

Consider the vorticity as defined by

{\boldsymbol {\omega }}=\nabla \times {\boldsymbol {u}}.

From the definition of the curl in spherical coordinates:

{\begin{aligned}\omega _{r}&={1 \over r\sin \theta }\left({\partial  \over \partial \theta }\left(u_{\phi }\sin \theta \right)-{\partial u_{\theta } \over \partial \phi }\right){\boldsymbol {\hat {r}}},\\\omega _{\theta }&={1 \over r}\left({1 \over \sin \theta }{\partial u_{r} \over \partial \phi }-{\partial  \over \partial r}\left(ru_{\phi }\right)\right){\boldsymbol {\hat {\theta }}},\\\omega _{\phi }&={1 \over r}\left({\partial  \over \partial r}\left(ru_{\theta }\right)-{\partial u_{r} \over \partial \theta }\right){\boldsymbol {\hat {\phi }}}.\end{aligned}}

First notice that the $r$ and $\theta$ components are equal to 0. Secondly substitute $u_{r}$ and $u_{\theta }$ into $\omega _{\phi }.$ The result is:

{\begin{aligned}\omega _{r}&=0,\\\omega _{\theta }&=0,\\\omega _{\phi }&={1 \over r}\left({\partial  \over \partial r}\left(r\left(-{\frac {1}{r\sin \theta }}{\frac {\partial \Psi }{\partial r}}\right)\right)-{\partial  \over \partial \theta }\left({\frac {1}{r^{2}\sin \theta }}{\frac {\partial \Psi }{\partial \theta }}\right)\right).\end{aligned}}

Next the following algebra is performed:

{\begin{aligned}\omega _{\phi }&={1 \over r}\left(-{\frac {1}{\sin \theta }}\left({\partial  \over \partial r}\left({\frac {\partial \Psi }{\partial r}}\right)\right)-{\frac {1}{r^{2}}}{\partial  \over \partial \theta }\left({\frac {1}{\sin \theta }}{\frac {\partial \Psi }{\partial \theta }}\right)\right)\\&={1 \over r}\left(-{\frac {1}{\sin \theta }}\left({\frac {\partial ^{2}\Psi }{\partial r^{2}}}\right)-{\frac {\sin \theta }{r^{2}\sin \theta }}{\partial  \over \partial \theta }\left({\frac {1}{\sin \theta }}{\frac {\partial \Psi }{\partial \theta }}\right)\right)\\&=-{\frac {1}{r\sin \theta }}\left({\frac {\partial ^{2}\Psi }{\partial r^{2}}}+{\frac {\sin \theta }{r^{2}}}{\partial  \over \partial \theta }\left({\frac {1}{\sin \theta }}{\frac {\partial \Psi }{\partial \theta }}\right)\right).\end{aligned}}

As a result, from the calculation the vorticity vector is found to be equal to:

{\boldsymbol {\omega }}={\begin{pmatrix}0\\[1ex]0\\[1ex]\displaystyle -{\frac {1}{r\sin \theta }}\left({\frac {\partial ^{2}\Psi }{\partial r^{2}}}+{\frac {\sin \theta }{r^{2}}}{\partial  \over \partial \theta }\left({\frac {1}{\sin \theta }}{\frac {\partial \Psi }{\partial \theta }}\right)\right)\end{pmatrix}}.

Comparison with cylindrical

The cylindrical and spherical coordinate systems are related through

z=r\,\cos \theta \,

and

\rho =r\,\sin \theta .\,

Alternative definition with opposite sign

As explained in the general stream function article, definitions using an opposite sign convention – for the relationship between the Stokes stream function and flow velocity – are also in use.[3]

Zero divergence

In cylindrical coordinates, the divergence of the velocity field u becomes:[4]

{\begin{aligned}\nabla \cdot {\boldsymbol {u}}&={\frac {1}{\rho }}{\frac {\partial }{\partial \rho }}{\Bigl (}\rho \,u_{\rho }{\Bigr )}+{\frac {\partial u_{z}}{\partial z}}\\&={\frac {1}{\rho }}{\frac {\partial }{\partial \rho }}\left(-{\frac {\partial \Psi }{\partial z}}\right)+{\frac {\partial }{\partial z}}\left({\frac {1}{\rho }}{\frac {\partial \Psi }{\partial \rho }}\right)=0,\end{aligned}}

as expected for an incompressible flow.

And in spherical coordinates:[5]

{\begin{aligned}\nabla \cdot {\boldsymbol {u}}&={\frac {1}{r\,\sin \theta }}{\frac {\partial }{\partial \theta }}(u_{\theta }\,\sin \theta )+{\frac {1}{r^{2}}}{\frac {\partial }{\partial r}}{\Bigl (}r^{2}\,u_{r}{\Bigr )}\\&={\frac {1}{r\,\sin \theta }}{\frac {\partial }{\partial \theta }}\left(-{\frac {1}{r}}{\frac {\partial \Psi }{\partial r}}\right)+{\frac {1}{r^{2}}}{\frac {\partial }{\partial r}}\left({\frac {1}{\sin \theta }}{\frac {\partial \Psi }{\partial \theta }}\right)=0.\end{aligned}}

Streamlines as curves of constant stream function

From calculus it is known that the gradient vector $\nabla \Psi$ is normal to the curve $\Psi =C$ (see e.g. Level set#Level sets versus the gradient). If it is shown that everywhere ${\boldsymbol {u}}\cdot \nabla \Psi =0,$ using the formula for ${\boldsymbol {u}}$ in terms of $\Psi ,$ then this proves that level curves of $\Psi$ are streamlines.

Cylindrical coordinates

In cylindrical coordinates,

\nabla \Psi ={\partial \Psi  \over \partial \rho }{\boldsymbol {e}}_{\rho }+{\partial \Psi  \over \partial z}{\boldsymbol {e}}_{z}

.

and

{\boldsymbol {u}}=u_{\rho }{\boldsymbol {e}}_{\rho }+u_{z}{\boldsymbol {e}}_{z}=-{1 \over \rho }{\partial \Psi  \over \partial z}{\boldsymbol {e}}_{\rho }+{1 \over \rho }{\partial \Psi  \over \partial \rho }{\boldsymbol {e}}_{z}.

So that

\nabla \Psi \cdot {\boldsymbol {u}}={\partial \Psi  \over \partial \rho }(-{1 \over \rho }{\partial \Psi  \over \partial z})+{\partial \Psi  \over \partial z}{1 \over \rho }{\partial \Psi  \over \partial \rho }=0.

Spherical coordinates

And in spherical coordinates

\nabla \Psi ={\partial \Psi  \over \partial r}{\boldsymbol {e}}_{r}+{1 \over r}{\partial \Psi  \over \partial \theta }{\boldsymbol {e}}_{\theta }

and

{\boldsymbol {u}}=u_{r}{\boldsymbol {e}}_{r}+u_{\theta }{\boldsymbol {e}}_{\theta }={1 \over r^{2}\sin \theta }{\partial \Psi  \over \partial \theta }{\boldsymbol {e}}_{r}-{1 \over r\sin \theta }{\partial \Psi  \over \partial r}{\boldsymbol {e}}_{\theta }.

So that

\nabla \Psi \cdot {\boldsymbol {u}}={\partial \Psi  \over \partial r}\cdot {1 \over r^{2}\sin \theta }{\partial \Psi  \over \partial \theta }+{1 \over r}{\partial \Psi  \over \partial \theta }\cdot {\Big (}-{1 \over r\sin \theta }{\partial \Psi  \over \partial r}{\Big )}=0.

Notes

Batchelor (1967), p. 78.
Batchelor (1967), p. 79.
E.g. Brenner, Howard (1961). "The slow motion of a sphere through a viscous fluid towards a plane surface". Chemical Engineering Science. 16 (3–4): 242–251. doi:10.1016/0009-2509(61)80035-3.
Batchelor (1967), p. 602.
Batchelor (1967), p. 601.

References

Batchelor, G.K. (1967). An Introduction to Fluid Dynamics. Cambridge University Press. ISBN 0-521-66396-2.
Lamb, H. (1994). Hydrodynamics (6th ed.). Cambridge University Press. ISBN 978-0-521-45868-9. Originally published in 1879, the 6th extended edition appeared first in 1932.
Stokes, G.G. (1842). "On the steady motion of incompressible fluids". Transactions of the Cambridge Philosophical Society. 7: 439–453. Bibcode:1848TCaPS...7..439S.
Reprinted in: Stokes, G.G. (1880). Mathematical and Physical Papers, Volume I. Cambridge University Press. pp. 1–16.

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[1] Batchelor (1967), p. 78.

[2] Batchelor (1967), p. 79.

[3] E.g. Brenner, Howard (1961). "The slow motion of a sphere through a viscous fluid towards a plane surface". Chemical Engineering Science. 16 (3–4): 242–251. doi:10.1016/0009-2509(61)80035-3.

[4] Batchelor (1967), p. 602.

[5] Batchelor (1967), p. 601.