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Stokes drift
For a pure wave motion in fluid dynamics, the Stokes drift velocity is the average velocity when following a specific fluid parcel as it travels with the fluid flow. For instance, a particle floating at the free surface of water waves, experiences a net Stokes drift velocity in the direction of wave propagation.
More generally, the Stokes drift velocity is the difference between the average Lagrangian flow velocity of a fluid parcel, and the average Eulerian flow velocity of the fluid at a fixed position. This nonlinear phenomenon is named after George Gabriel Stokes, who derived expressions for this drift in his 1847 study of water waves.
The Stokes drift is the difference in end positions, after a predefined amount of time (usually one wave period), as derived from a description in the Lagrangian and Eulerian coordinates. The end position in the Lagrangian description is obtained by following a specific fluid parcel during the time interval. The corresponding end position in the Eulerian description is obtained by integrating the flow velocity at a fixed position—equal to the initial position in the Lagrangian description—during the same time interval.
The Stokes drift velocity equals the Stokes drift divided by the considered time interval. Often, the Stokes drift velocity is loosely referred to as Stokes drift. Stokes drift may occur in all instances of oscillatory flow which are inhomogeneous in space. For instance in water waves, tides and atmospheric waves.
In the Lagrangian description, fluid parcels may drift far from their initial positions. As a result, the unambiguous definition of an average Lagrangian velocity and Stokes drift velocity, which can be attributed to a certain fixed position, is by no means a trivial task. However, such an unambiguous description is provided by the Generalized Lagrangian Mean (GLM) theory of Andrews and McIntyre in 1978.^{[1]}
The Stokes drift is important for the mass transfer of all kind of materials and organisms by oscillatory flows. Further the Stokes drift is important for the generation of Langmuir circulations.^{[2]} For nonlinear and periodic water waves, accurate results on the Stokes drift have been computed and tabulated.^{[3]}
Contents
Mathematical description
The Lagrangian motion of a fluid parcel with position vector x = ξ(α,t) in the Eulerian coordinates is given by:^{[4]}
 <math>
\dot{\boldsymbol{\xi}}\, =\, \frac{\partial \boldsymbol{\xi}}{\partial t}\, =\, \boldsymbol{u}(\boldsymbol{\xi},t),
</math> where ∂ξ / ∂t is the partial derivative of ξ(α,t) with respect to t, and
 ξ(α,t) is the Lagrangian position vector of a fluid parcel, in meters,
 u(x,t) is the Eulerian velocity, in meters per second,
 x is the position vector in the Eulerian coordinate system, in meters,
 α is the position vector in the Lagrangian coordinate system, in meters,
 t is the time, in seconds.
Often, the Lagrangian coordinates α are chosen to coincide with the Eulerian coordinates x at the initial time t = t_{0} :^{[4]}
 <math>
\boldsymbol{\xi}(\boldsymbol{\alpha},t_0)\, =\, \boldsymbol{\alpha}.
</math> But also other ways of labeling the fluid parcels are possible.
If the average value of a quantity is denoted by an overbar, then the average Eulerian velocity vector ū_{E} and average Lagrangian velocity vector ū_{L} are:
 <math>
\begin{align} \overline{\boldsymbol{u}}_E\, &=\, \overline{\boldsymbol{u}(\boldsymbol{x},t)}, \\ \overline{\boldsymbol{u}}_L\, &=\, \overline{\dot{\boldsymbol{\xi}}(\boldsymbol{\alpha},t)}\, =\, \overline{\left(\frac{\partial \boldsymbol{\xi}(\boldsymbol{\alpha},t)}{\partial t}\right)}\, =\, \overline{\boldsymbol{u}(\boldsymbol{\xi}(\boldsymbol{\alpha},t),t)}. \end{align}
</math> Different definitions of the average may be used, depending on the subject of study, see ergodic theory:
 time average,
 space average,
 ensemble average and
 phase average.
Now, the Stokes drift velocity ū_{S} equals^{[5]}
 <math>
\overline{\boldsymbol{u}}_S\, =\, \overline{\boldsymbol{u}}_L\, \, \overline{\boldsymbol{u}}_E.
</math> In many situations, the mapping of average quantities from some Eulerian position x to a corresponding Lagrangian position α forms a problem. Since a fluid parcel with label α traverses along a path of many different Eulerian positions x, it is not possible to assign α to a unique x. A mathematically sound basis for an unambiguous mapping between average Lagrangian and Eulerian quantities is provided by the theory of the Generalized Lagrangian Mean (GLM) by Andrews and McIntyre (1978).
Example: A onedimensional compressible flow
For the Eulerian velocity as a monochromatic wave of any nature in a continuous medium: <math>u=\hat{u}\sin\left( kx  \omega t \right),</math> one readily obtains by the perturbation theory – with <math>k\hat{u}/\omega</math> as a small parameter – for the particle position <math>x=\xi(\xi_0,t):</math>
 <math>\dotTemplate:\xi=\, {u}({\xi},t)= \hat{u} \sin\, \left( k \xi  \omega t \right),</math>
 <math>
\xi(\xi_0,t)\approx\xi_0+\frac{\hat{u}}{\omega}\cos(k\xi_0\omega t)+\frac{k\hat{u}^2}{2\omega^2}\sin2(k\xi_0\omega t)+\frac{k\hat{u}^2}{2\omega} t.
</math> Here the last term describes the Stokes drift <math>\tfrac12 k\hat{u}^2/\omega.</math>^{[6]}
Example: Deep water waves
The Stokes drift was formulated for water waves by George Gabriel Stokes in 1847. For simplicity, the case of infinitedeep water is considered, with linear wave propagation of a sinusoidal wave on the free surface of a fluid layer:^{[7]}
 <math>
\eta\, =\, a\, \cos\, \left( k x  \omega t \right),
</math> where
 η is the elevation of the free surface in the zdirection (meters),
 a is the wave amplitude (meters),
 k is the wave number: k = 2π / λ (radians per meter),
 ω is the angular frequency: ω = 2π / T (radians per second),
 x is the horizontal coordinate and the wave propagation direction (meters),
 z is the vertical coordinate, with the positive z direction pointing out of the fluid layer (meters),
 λ is the wave length (meters), and
 T is the wave period (seconds).
As derived below, the horizontal component ū_{S}(z) of the Stokes drift velocity for deepwater waves is approximately:^{[8]}
<math>
\overline{u}_S\, \approx\, \omega\, k\, a^2\, \text{e}^{2 k z}\, =\, \frac{4\pi^2\, a^2}{\lambda\, T}\, \text{e}^{4\pi\, z / \lambda}.
</math>
As can be seen, the Stokes drift velocity ū_{S} is a nonlinear quantity in terms of the wave amplitude a. Further, the Stokes drift velocity decays exponentially with depth: at a depth of a quart wavelength, z = ¼ λ, it is about 4% of its value at the mean free surface, z = 0.
Derivation
It is assumed that the waves are of infinitesimal amplitude and the free surface oscillates around the mean level z = 0. The waves propagate under the action of gravity, with a constant acceleration vector by gravity (pointing downward in the negative zdirection). Further the fluid is assumed to be inviscid^{[9]} and incompressible, with a constant mass density. The fluid flow is irrotational. At infinite depth, the fluid is taken to be at rest.
Now the flow may be represented by a velocity potential φ, satisfying the Laplace equation and^{[7]}
 <math>
\varphi\, =\, \frac{\omega}{k}\, a\; \text{e}^{k z}\, \sin\, \left( k x  \omega t \right).
</math> In order to have nontrivial solutions for this eigenvalue problem, the wave length and wave period may not be chosen arbitrarily, but must satisfy the deepwater dispersion relation:^{[10]}
 <math>
\omega^2\, =\, g\, k.
</math> with g the acceleration by gravity in (m / s^{2}). Within the framework of linear theory, the horizontal and vertical components, ξ_{x} and ξ_{z} respectively, of the Lagrangian position ξ are:^{[8]}
 <math>
\begin{align} \xi_x\, &=\, x\, +\, \int\, \frac{\partial \varphi}{\partial x}\; \text{d}t\, =\, x\, \, a\, \text{e}^{k z}\, \sin\, \left( k x  \omega t \right), \\ \xi_z\, &=\, z\, +\, \int\, \frac{\partial \varphi}{\partial z}\; \text{d}t\, =\, z\, +\, a\, \text{e}^{k z}\, \cos\, \left( k x  \omega t \right). \end{align}
</math> The horizontal component ū_{S} of the Stokes drift velocity is estimated by using a Taylor expansion around x of the Eulerian horizontalvelocity component u_{x} = ∂ξ_{x} / ∂t at the position ξ :^{[4]}
 <math>
\begin{align} \overline{u}_S\, &=\, \overline{u_x(\boldsymbol{\xi},t)}\, \, \overline{u_x(\boldsymbol{x},t)}\,
\\ &=\, \overline{\left[ u_x(\boldsymbol{x},t)\, +\, \left( \xi_x  x \right)\, \frac{\partial u_x(\boldsymbol{x},t)}{\partial x}\, +\, \left( \xi_z  z \right)\, \frac{\partial u_x(\boldsymbol{x},t)}{\partial z}\, +\, \cdots \right] } \, \overline{u_x(\boldsymbol{x},t)} \\ &\approx\, \overline{\left( \xi_x  x \right)\, \frac{\partial^2 \xi_x}{\partial x\, \partial t} }\, +\, \overline{\left( \xi_z  z \right)\, \frac{\partial^2 \xi_x}{\partial z\, \partial t} } \\ &=\, \overline{ \bigg[  a\, \text{e}^{k z}\, \sin\, \left( k x  \omega t \right) \bigg]\, \bigg[ \omega\, k\, a\, \text{e}^{k z}\, \sin\, \left( k x  \omega t \right) \bigg] }\, \\ &+\, \overline{ \bigg[ a\, \text{e}^{k z}\, \cos\, \left( k x  \omega t \right) \bigg]\, \bigg[ \omega\, k\, a\, \text{e}^{k z}\, \cos\, \left( k x  \omega t \right) \bigg] }\, \\ &=\, \overline{ \omega\, k\, a^2\, \text{e}^{2 k z}\, \bigg[ \sin^2\, \left( k x  \omega t \right) + \cos^2\, \left( k x  \omega t \right) \bigg] } \\ &=\, \omega\, k\, a^2\, \text{e}^{2 k z}. \end{align}
</math>
See also
References
Historical
 A.D.D. Craik (2005). "George Gabriel Stokes on water wave theory". Annual Review of Fluid Mechanics 37: 23–42. Bibcode:2005AnRFM..37...23C. doi:10.1146/annurev.fluid.37.061903.175836.
 G.G. Stokes (1847). "On the theory of oscillatory waves". Transactions of the Cambridge Philosophical Society 8: 441–455.
Reprinted in: G.G. Stokes (1880). Mathematical and Physical Papers, Volume I. Cambridge University Press. pp. 197–229.
Other
 D.G. Andrews and M.E. McIntyre (1978). "An exact theory of nonlinear waves on a Lagrangian mean flow". Journal of Fluid Mechanics 89 (4): 609–646. Bibcode:1978JFM....89..609A. doi:10.1017/S0022112078002773.
 A.D.D. Craik (1985). Wave interactions and fluid flows. Cambridge University Press. ISBN 0521368294.
 M.S. LonguetHiggins (1953). "Mass transport in water waves". Philosophical Transactions of the Royal Society A 245 (903): 535–581. Bibcode:1953RSPTA.245..535L. doi:10.1098/rsta.1953.0006.
 Phillips, O.M. (1977). The dynamics of the upper ocean (2nd ed.). Cambridge University Press. ISBN 0521298016.
 G. Falkovich (2011). Fluid Mechanics (A short course for physicists). Cambridge University Press. ISBN 9781107005754.
Notes
 ↑ See Craik (1985), page 105–113.
 ↑ See e.g. Craik (1985), page 120.
 ↑ Solutions of the particle trajectories in fully nonlinear periodic waves and the Lagrangian wave period they experience can for instance be found in:
J.M. Williams (1981). "Limiting gravity waves in water of ﬁnite depth". Philosophical Transactions of the Royal Society A 302 (1466): 139–188. Bibcode:1981RSPTA.302..139W. doi:10.1098/rsta.1981.0159.
J.M. Williams (1985). Tables of progressive gravity waves. Pitman. ISBN 9780273087335.  ↑ ^{4.0} ^{4.1} ^{4.2} See Phillips (1977), page 43.
 ↑ See e.g. Craik (1985), page 84.
 ↑ See Falkovich (2011), pages 71–72.
 ↑ ^{7.0} ^{7.1} See e.g. Phillips (1977), page 37.
 ↑ ^{8.0} ^{8.1} See Phillips (1977), page 44. Or Craik (1985), page 110.
 ↑ Viscosity has a pronounced effect on the mean Eulerian velocity and mean Lagrangian (or mass transport) velocity, but much less on their difference: the Stokes drift outside the boundary layers near bed and free surface, see for instance LonguetHiggins (1953). Or Phillips (1977), pages 53–58.
 ↑ See e.g. Phillips (1977), page 38.
