complete set of the shallow water equations:
\(u_t-fv=-g\eta_x \\ v_t+fu=-g\eta_y \\ \eta_t+H(u_x+v_y)=0\)
derivation:
1. hydrostatic approximation: \( .\\ (\frac{H}{L})^2<<1\\ \)
2. horizontal momentum equations for small perturbations about a state of rest (working with total pressure):
\(u_t-fv=-\frac{p_x}{p_0} \\ v_t +fu=-\frac{p_y}{p_0}\)
3. hydrostatic equation:
\(0=-\frac{\partial p}{\partial z}-g\rho_0 \\ =>p=p_a+g\rho_0(\eta-z) \\ =>p_x=(p_a)_x+g\rho_0\eta_x\)
it follows:
\(u_t-fv=-g\eta_x-(\frac{p_{ax}}{\rho_0}) \\ v_t-fu=-g\eta_y-(\frac{p_{ay}}{\rho_0})\)
3. the kinematic boundary condition at the sea surface:
the total change of sea surface height is äquivalent to the vertical motion w:
\(\eta_t+u\eta_x+v\eta_y=w\)
for small perturbations about a state of rest it follows:
\(\eta_t=w\)
4. integrating the continuity equation and applying \(\eta_t=0\) yields:
\(\int_{-H}^{0}(u_x+v_y)\;dz=-\int_{-H}^{0}w_z\;dz=-\eta_t \\ => \eta_t+H(u_x+v_y)=0\)
5. assuming uniform atmospheric pressure:
\(i.e.\;\;p_{ax}=p_{ay}=0\)
What is the main concept of a layer model?
S.262
What is the rigid-lid approximation? \(p_a\)
The upper boundary condition of the ocean model is moved from the free surface \(z=\zeta\) to a flat surface \(z=0\).
If we assume the lowest layer to be stagnant then this leads to a drop out of the atmospheric pressure in the horizontal pressure gradient terms.
\(p_a=p_{a,0}+\rho g \zeta\)
This leads for the 1 1/2-layer model again to the shallow water equations:
\(u_t-fv= -g'h_x \\ v_t+fu=-g'h_y \\ h_t+H_1(u_x+v_y)=0\)
g' is the reduced gravity:
\(g'=g(\rho_1-\rho_2)/\rho_0\)
Explain the meridional flow driven by Ekman pumping.
=> Ekman pumping in the subtropical basin drives an equatorward flow in the ocean interior.
=> Ekman upwelling in the subpolar basin drives a poleward flow in the ocean interior.
figure in Huang et al. 2010 S.286
Including wind forcing to the shallow water equations!
\(u_t-fv=-\frac{p'_x}{\rho_0}+\frac{\partial X}{\partial z} \\ v_t+fu=-\frac{p'_y}{\rho_0}+\frac{\partial Y}{\partial z}\)
with
\(X=\nu u_z,\;\;Y=\nu v_z\)
where \(\nu \) is a vertical eddy viscosity (but could also be something else)
The connection between vertical eddy viscosity and the surface wind stress is:
\(\nu u_z=\tau^x_s/\rho_0\;\;\;\nu v_z=\tau^y_s/\rho_0\)
This means: \(\rho_0(X,Y)\) is the horizontally acting stress at each depth
In this course we often set:
\(\nu=\left\{ \begin{array}{c} \nu_0\;\;\;for\;-H_E\leq z\leq0\\0\;\;\; otherwise \end{array} \right.\)
The balance
\(-fv=(\nu u_z)_z\\fu=(\nu v_z)_z\)
implies, for uniform \(\nu\) the scaling
\(fU=\frac{\nu U}{h^2}=>h=\sqrt{\frac{\nu}{f}}\) (h is the vertical scale)
i.e. for uniform \(\nu\) variations in the vertical take place in a scale \(\sqrt{\frac{\nu}{f}}\) . If this scale is much larger than the depth over which \(\nu\) is non-zero, then the horizontal velocity will be essentially independent of depth over the region where \(\nu\) is non-zero, in this case the depth \(H_E\) .
For this case we can treat wind stress as a body force over the depth \(H_E\) . Which means the wind stress forcing is constant for each layer whithin the Ekman Layer.
\(\left(\frac{\partial X}{\partial z},\frac{\partial Y}{\partial z}\right)=\frac{G(z)}{\rho_0H_E}(\tau_s^x,\tau^y_s)\)
with
\(G(z)=\left\{ \begin{array}{c} 1\;\;-H_E\leq z\leq0\\0\;\;otherwise \end{array} \right.\)
for the 1 1/2 layer model follows with wind forcing:
\(u_t-fv=-g'h_x+\frac{\tau^x_s}{\rho_1H_1}\\v_t+fu=-g'h_y+\frac{\tau_s^y}{\rho_1H_1}\\h_t+H_1(u_x+v_y)=0\)
Ekman dynamics!
Consider the Ekman part of the flow:
\(u_t-fv=-\frac{p'_x}{\rho_0}+\frac{\partial X}{\partial z}\\ v_t+fu=-\frac{p'_y}{\rho_0}+\frac{\partial Y}{\partial z}\)
is going to:
\(u_t-fv=+\frac{\partial X}{\partial z}\\ v_t+fu=-\frac{\partial Y}{\partial z}\)
1. Assuming that the flow is al confined above a depth \(H_E\) , the EKMAN TRANSPORT, (\((U_E,V_E)\), is defined as:
\((U_E,V_E)=\int\limits_{-H_E}^0(u_E,v_E)dz\)
\((u_E,v_E) \)i is the Ekman Velocity.
2. Assuming \((X,Y)=0\)below the Ekman depth, it follows that
\(U_{Et}-fV_E=\frac{\tau^x_s}{\rho_0H_E}\\V_{Et}+fU_E=\frac{\tau^y_s}{\rho_0H_E}\)
-> In steady state, the Ekman transport is at right angles to the surface wind stress, i.e.
\(-fV_E=\frac{\tau^x_s}{\rho_0H_E}\\fU_E=\frac{\tau^x_s}{\rho_0H_E}\)
Geostrophic dynamics: What says the Taylor-Proudman Theorem?
The geostrophic balance is expressed by:
\(-fv_g=-\frac{1}{\rho_0}p_x\\ fu_g=-\frac{1}{\rho_0}P_y\)
where \((u_g,v_g)\) is the geostrophic flow. It follows that:
\(\frac{\partial u_g}{\partial x}+\frac{\partial v_g}{\partial y}=-\frac{\beta v}{f}\)
On a f-plane, \(\beta=0\) and hence
\(\frac{\partial u_g}{\partial x}+\frac{\partial v_g}{\partial y}=0\)
Using \(u_x+v_y+w_z=0 \) it follows for the f-plane:
\(w_z=0\)
This means that if vertical velocity is somewhere zero (as it is for the bottom the case), than it is everywhere zero! It follows that flow will tend to go around topography and not over topography!
Furthermore, with the thermal wind equations it can be shown that for a fluid with uniform density, that there is no variation in the geostrophic flow in the vertical (no geostrophic shear!) which means that above a bump, the flow will be stagnant at all depths!
The Taylor-Proudman Theorem states that flow tends to go around bumps rather than over them!
Write down the thermal wind equations!
Combine the geostrophic balance
\(-fv=-\frac{1}{\rho_0}p_x\\fu=-\frac{1}{\rho_0}p_y\)
with the hydrostatic balance \(0=-p_z-g\rho\) to give
\(fv_z=-\frac{g}{\rho_0}\rho_x\\fu_z=\frac{g}{\rho_0}\rho_y\)
Give the equation for the linear vorticity balance and explain it!
The steady-state zonal and meridional momentum equations (linearised about a state of rest) are:
\(-fv=-\frac{1}{\rho_0}p_x+\frac{\tau^x_s}{\rho_0H_E}G(z)\\ fu=-\frac{1}{\rho_0}p_y+\frac{\tau^y_s}{\rho_0H_E}G(z)\)
Taking \(\frac{\partial 2}{\partial x}-\frac{\partial 1}{\partial y}\) and using \(u_x+v_y+w_z=0\) gives
\(\beta v=fw_z+\frac{G(z)}{\rho_0H_E}[\frac{\partial \tau^y_s}{\partial x}-\frac{\partial \tau^x_s}{\partial y}]\)
\(\beta v\) ...advection of planetary vorticity
\(fw_z\) ...vortex stretching -> locally stretching \((w_z>0)\)leads to an increase of vorticity and likewise
\(\frac{G(z)}{\rho_0H_E}[\frac{\partial \tau^y_s}{\partial x}-\frac{\partial \tau^x_s}{\partial y}]\)...vorticity input by the curl of the surface wind stress
Give the Sverdrup relation.
If we set for the linear vorticity equation wind stress zero, then we get the Sverdrup relation:
\(\beta v=fw_z\)
By vertically integrating we can gain the conservation of potential vorticity:
layers of uniform density: \(\frac{D}{Dt}\frac{f}{h}=0\)
continuous stratification: \(\frac{D}{Dt}[f\rho_z]=0\)
Sketch the Stommel Model! (alt)
we start from a flat-bottomed ocean with uniform density. The linearized equations of motions for a steady flow are:
\(-fv=-g\eta_x+(vu_z)_z\\ fu=-g\eta_y+(vv_z)_z\\ u_x+v_y+w_z=0\)
vertical averaging and paramterization of the bottom stressin terms of the vertical averaged flow brings:
\(-f\bar{v}=-g\eta_x+\frac{\tau_s^x}{\rho_0H}-\frac{r\bar{u}}{H}\\ f\bar{u}=-g\eta_y+\frac{\tau_s^y}{\rho_0 H}-\frac{r\bar{v}}{H}\)
since \((\bar{u}H)_x+(\bar{v}H)_y=0\) ,there exists a streamfunction
Taking \(\frac{\partial }{\partial x}(2)-\frac{\partial }{\partial y}(2)\) gives
\(.\\ \frac{r}{H}[\frac{\partial \bar{v}}{\partial x}-\frac{\partial \bar{u}}{\partial y}]+\beta\bar{v}=\frac{1}{\rho_0H}[\frac{\partial }{\partial x}(\tau_s^y)-\frac{\partial }{\partial y} (\tau_s^x)]\)
or as stream function: \(\gamma \nabla^2\Psi+\beta \Psi_x=F\)
where \(\gamma=\frac{r}{H}\) is the friction parameter and \(F=\frac{1}{\rho_0}[\frac{\partial }{\partial x}(\tau_s^y)-\frac{\partial }{\partial y} (\tau_s^x)]\) is the curl of the wind stress.
Coming to the model geometry:
x=0 ... western boundary; x=\(\alpha\)L ... eastern boundary
\(y=y_0\)... runs across the middle of the domain.
Parameterization of the surface wind stress:
\(\tau_s^x=\tau_0sin(\frac{y-y_0}{L})\\ \tau_s^y=0\)
it follows: \(F=-\frac{1}{\rho_0}[\frac{\tau_0}{L}cos(\frac{y-y_0}{L})]\)
Seek a solution of the form \(\Psi=\psi(x)cos(\frac{y-y_0}{L})\) where \(\psi=\psi(x)\) . Then
\(-\frac{\gamma}{L^2}\psi+\gamma \frac{d^2\psi}{dx^2}+\beta\frac{d\psi}{dx}=-\frac{\tau_0}{\rho_0L}\)
We now can non-dimensionalise the equation by defining: \(x'=x/L\) and \(\psi'=\frac{\psi}{\tau_0/(\rho_0\beta)}\) . Then:
Quasi-Geostrophic Dynamics: Derive and discuss the quasi-geostrophic equations for a (non-linear) \(1\frac{1}{2}\) layer model.
The governing equations are:
Since we aspect the dominant balance to be geostrophy, i.e.
\(-fv=-g'h_x\\fu=-g'h_y\)
this suggests: \(f_0U=\frac{g'D}{L}\)
Now non-dimensionalise as follows:
\(u,v \leftrightarrow U\\x,y\leftrightarrow L\\t\leftrightarrow T\\\tau_s^x,\tau_s^y\leftrightarrow\tau_0\\h\leftrightarrow \frac{f_0UL}{g'}\)
The non-dimensionalising brings the following:
\(\epsilon_Tu_t+R_0(uu_x+vu_y)-(1+\epsilon_\beta y)v=-h_x+\frac{\epsilon_E\tau_s^x}{(1+FR_0h)}\\\epsilon_Tv_t+R_0(uv_x+vv_y)-(1+\epsilon_\beta y)u=-h_y+\frac{\epsilon_E\tau_s^y}{(1+FR_0h)}\)
where
\(\epsilon_T=\frac{1}{f_0T}\;\;\;\epsilon_\beta=\frac{\beta L}{f_0}\\R_0=\frac{U}{f_0L}\;\;(Rossby\;number)\\\epsilon_E=\frac{\tau_0}{\rho_0H_1f_0U}\;\;(Ekman\;number)\\F=(\frac{L}{R})^2\;\;where\;\;R=\frac{c}{f_0}\;(radius\;of\;deformation)\;\;c=\sqrt{g'H_1}\)
For geostrophic balance we assume: \(F\approx1\;and\;\epsilon_T=R_0=\epsilon_\beta =\epsilon_E=\epsilon\ll1\)
At lowest order in \(\epsilon\), we have \(u=u_g,\;v=v_g\)
The full velocity is then (with the additional 4 parts):
\(u=u_g+\epsilon u_a\\v=v_g+\epsilon v_a\)
where \(\epsilon u_a\;and\;\epsilon v_a\) is the ageostrophic flow.
The ageostrophic part of the \(U=U_g+U_a\)velocity , approximated all terms of order 1 in respect to \(\epsilon\) , is
back to the dimensionalized form:
\(f_0u_a=-\beta yu_g-v_{gt}-(u_gv_{gx}+v_gv_{gy})+\frac{\tau_s^y}{\rho_0H_1}\\f_0v_a=-\beta yv_g+u_{gt}+(u_gu_{gx}+v_gu_{gy})+\frac{\tau_s^x}{\rho_0H_1}\)
What is the advantage of reduced gravity models?
The wind-driven circulation has been described in terms of the quasi-geostrophic model derived from the shallow water equation in many textbooks.
Although, the wind-driven gyres in mid latitudes have horizontal scales much larger than the synoptic scale assumed in the quasi-geostrophic approximation.
As a result, one of the basic assumptions in the traditional quasi-gesostrophic approximation , that deviations from the mean stratification are small, is no longer valid.
Although the quasi-geostrophic theory remains a useful tool for describing the circulation, the strong nonlinearity due to the meridional change of stratification can be handled much more accurately by using simple reduced-gravity models.
Why do we need a western boundary?
The wind-driven circulation in the ocean interior can be described in terms of the balance between the Coriolis force, the pressure gradient and the wind stress.
From both the energy and potential vorticity equations, it is clear that a purely inertial western boundary current cannot satisfy the energy and potential vorticity balance in a closed basin. No matter how small the friction is, it plays an essential role in balancing the energy and potential vorticity in a closed basin by dissipating the potential vorticity and energy input from the wind stress.
The following models for the western boundary do exist:
Explain the interior solution.
Assumptions:
the momentum equations are reduced to:
\(-fhv=-g'hh_x+\tau^x/\rho_0\\ fhu=-g'hh_y\)
Cross-differentiating and subtraction leads to the vorticity equation:
\(\beta hv=-\tau^x_y/\rho_0 \)
This equation is called the Sverdrup relation!
Substituting the Sverdrup relation back to the first moemntum equation gives the first-order ordinary differential equation:
\(hh_x=-\frac{f^2}{g'\rho_0\beta}(\frac{\tau^x}{f})_y\)
Integrating this leads to the interior solution. To start the integration we need to choose the eastern boundary to balance the vorticity in the basin.
Using \(\psi_x=hv,\;\;\psi_y=-hu\) leads to:
\(\psi =\frac{1}{\rho_0 \beta}\tau_y^x(x_e-x)\)
This volume is called the Sverdrup transport!
Two results:
Common features of the Western boundary layer regardless to the specific dynamic balance assumptions (Stommel, Munk,...)
To a very good approximation the cross-stream pressure gradient is in balance with the Coriolis force associated with the downstream velocity.
However, the downstream momentum is in ageostrophic balance, i.e. the downstream momentum balance must include downstream pressure.
Thus, the boundary layer is said to be in semi-geostrophic balance.
Two important features for the general solution of the western boundary layer:
(Note that layer thickness in the reduced-gravity model can be interpreted as either pressure or free surface elevation.)
The Stommel boundary layer
Stommel (1948) made the assumption that interfacial friction is in the form of a linear drag law. Thus, within the western boundary layer the downstream momentum equation is in an ageostrophic balance
\(fhu=-g'hh_y-Rv\)
The dynamical balance of the circulation is best illustrated in terms of the potential vorticity change along closed streamlines. Since the relative vorticity is very small, the potential vorticity can be approximated by \((\Delta \rho /\rho_0)(f/h)\).
In the basin interior the wind-stress curl is a sink of potential vorticity; thus, potential vorticity declines downstream In the western boundary, the interfacial friction torque is a source of positive potential vorticity; thus, potential vorticity of a water parcel increases along the pathway.
In the basin interior, the interfrictional friction torque is negligible. Within the western boundary layer the wind-stress torque is negligible.
Similarly, the energy balance along streamlines consits of two stages. First, in the basin interior, wind stress imposes mechanical energy into the circulation, primarily near both the northern and southern boundaries, where the zonal velocity and wind stress are large. This external mechanical energy input is balanced by an energy sink due to interfacial friction.
Munk boundary layer.
Munk (1950) postulated that the lateral friction works as the major dissipation mechanism. Lateral friction is parameterized in terms of \(\nabla ^2_h(h\vec{u})\)
Therefore, the basic momentum equations are as follows:
\(-fhv=g'hh_x+A_h\nabla^2_h(hu)+\tau^x/\rho_0\\fhu=-g'hh_y+A_h\nabla_h^2(hv)\)
Explain the meridional flow by Ekan pumping physical!
Thus, Ekman pumping in the subtropical basin drives an equatorward flow in the ocean interior. Similarly, the Ekman upwelling in the subpolar basin drives a poleward flow in the ocean interior.
Explain the need of potential vorticity balance and why this can only be provided by a western boundary layer!
The problem: the interior solution is valid all the way up to the eastern wall; thus, the solution in the interior can be obtained by starting the integration from the eastern boundary. On the other hand, there is a western boundary layer, so we would not be able to obtain the interior solution by integration from the western boundary.
Explanation:
We are in the subtropical basin: Water continously gains negative vorticity from the upper boundary. The circulation in the ocean interior is very slow, and the relative vorticity is negligible; thus, water parcels move southward to a place where the planetary vorticity is smaller. To close the ciruclation, water needs to move northward at the western or eastern wall and gain vorticity.
-> No matter what kind of model we use, there should always be a place where positive vorticity is generated through either interfacial or lateral friction to counterbalance the vorticity input from wind-stress curl in the interior.
As the graphic shows, only a wall to the left side can provide positive vorticity input through friction. Therefore, only a western boundary current can play the role of balancing potential vorticity in a closed basin.
Reciruclation: What is the mitovation for a closer look?
Our discussion has been limited to models based on Sverdrup dynamic. The western boundary currents were just matched to the interior solution. Within this theoretical framework, the maximal streamfunction is totally determined by a zonal integration of the Ekman pumping velocity, started from the eastern boundary of the basin.
Observations, however, indicate that the maximal volume flux in the Gulf Stream is about 150Sv, which is several times larger than the value calculated from the Sverdrup relation.
The discrepancy between the linear theory and observations is due to two factors:
The JEBAR term
When the ocean bottom is not flat, the JEBAR term arises when the curl is taken of the vertically-averaged horizontal momentum equations.
In fact, JEBAR comes directly from taking the curl of the veritically-averaged horizontal pressure gradient term.
\(J(\Psi,\frac{f}{H})=J(\Phi,\frac{1}{H})+\frac{1}{\rho_0}[\frac{\partial }{\partial x}(\frac{\tau_s^y}{H})-\frac{\partial }{\partial y}(\frac{\tau_s^x}{H})]\)
The first term on the right-hand side is called the JEBAR term, and the second term on the right-hand side is the contribution due to wind-strss curl.
The equation states that changes of the barotropic streamfunction along the \(f/H\) contours are due to contributions from these two terms.
The JEBAR term is associated with bottom pressure torque, and is the result of interaction between the stratification and bottom topography. It can be readily seen that, for the case of a flat bottom, this terms vanishes.
Greatbatch et al. (1991) analyzed the circulation on the North Atlantic Ocean. The most crucial contributor to the volume transport in the recirculation regime is the JEBAR term.
Explain the essence of the quasi-geostrophic theory!
While geostrophic motion refers to the wind that would result from an exact balance between the Coriolis force and horizontal pressure-gradient forces,[1] quasi-geostrophic (QG) motion refers to flows where the Coriolis force and pressure gradient forces are almost in balance, but with inertia also having an effect.
This effect of inertia is reffered to the ageostrophic part of the velocity, which is under the following assumptions much smaller than the geostrophic part:
The most important implification is that vertical displacements are small compared to the background stratification!
Scale anaylsis for the \(1\frac{1}{2}\)-layer model
At highest order of simplification the flow is purely geostrophic:This means also that on a f-plane the flow is non-divergent.
To have vertical motion we need to consider the ageostrophic flow.
The ageostrophic flow has 4 parts:
Give the equation for the quasi-geostrophic potential Vorticity!
\(\psi \) is the quasi-geostrophic stream function.
\(\frac{D_g}{Dt}(\nabla^2\psi +\beta y-\frac{f_0^2}{c^2}\psi )=\frac{1}{\rho_0H_1}(\frac{\partial }{\partial x}\tau_s^y-\frac{\partial}{\partial y} \tau_s^x)\)
\(\nabla ^2 \psi \)... is the relative vorticity
\(f_0+\beta y\)... is the planetary vorticity
\(\frac{f_0^2}{c^2 }\psi\)... is the stretching term
\(\frac{\partial }{\partial x}\tau_s^y-\frac{\partial}{\partial y}\tau_s^x\)... is the wind stress curl
If the wind stress curl is 0 then:
\(\frac{D_q}{Dt}=0\;\;where\;\;q=\nabla^2\psi+\beta y-\frac{f_0^2}{c^2}\psi \)
q is the quasi-geostrophic potential vorticity;
\(\frac{Dq}{Dt}=0\) states the Conservation of Quasi-Geostrophic Potential Vorticity
If q is conserved, then changes of the planetary vorticity are balanced bx changes of the relative vorticity and vortex stretching.
What important assumption is made in the quasi-geostrophic theory?
It is assumed, that vertical displacements are not so large as to disturb the background stratification. In the \(1\frac{1}{2}\) layer model, this corresponds to the assumption that the interface displacements are small compared to the undisturbed depth \(H_1\).
Give the dispersion relation of linear Rossby Waves and explain the difference between long and short waves!
Under the assumption of conservation of the quasi-geostrophic potential vorticity \(Dq/Dt=0\) and a solution of the form:
\(\psi=\psi_0e^{i(kx+ly-\omega t)}\)
We find the dispersion relation:
\(\omega=-\frac{\beta k }{(k^2+l^2+\frac{f_0^2}{c^2})}\)
For fixed l the solution has the following form as shown in the graphic below.
long waves are: \(\frac{\partial \omega}{\partial k}<0 \) -> westward group velocity
short waves are: \(\frac{\partial \omega}{\partial k }>0\) -> eastward group velocity
Western intensification: short waves trapped near western boundary; long waves escape westwards.
Long Waves
The limit for the long waves is:
\(k^2+l^2<<\frac{f_0^2}{c^2}\)
... horizontal length scales are much larger than the radius of deformation
for long waves the dispersion relation reduces to:
\(\omega =-\beta\frac{c^2}{f_0^2}k\)
-> These waves are non-dispersive with westward phase and group velocity given by \(\beta\frac{c^2}{f_0^2}\).
thinking of the shallow water equations:
\(u_t-fv=-g'h_x\\ v_t+fu=-g'h_y\\ h_t+H_1(u_x+v_y)=0\)
The long wave limit is equivalent to neglecting \(u_t,v_t\) and so:
\(h_t-\frac{\beta g'H_1}{f^2}h_x=0\;\;with\;\;\beta=\frac{df}{dy}\)
assuming wave solution \(h=h_0e^{i(\omega t-kx-ly)}\) we get to the dispersion relation (see above).
Divergence of the ageostrophic flow due to \(\beta\) is balanced by "vortex stretching", i.e. pumps the thermocline up and down via the \(h_t \) term.
To cross the North Atlantic Ocean, these waves need roughly 25 years! Although the propagation speed increases toward equator, where it takes only 1 year.
Short Waves
The limit of short waves is:
\(k^2+l^2>>\frac{f_0^2}{c^2}\)
-> length scales are much smaller than the Radius of Deformation!
Usually appropriate for the barotropic mode in the ocean: \(c=200m/s\)
The dispersion relation reduces to:
\(\omega=-\frac{\beta k}{(k^2+l^2)}\)
These waves are highly dispersive (the phase and group velocity are far from being equal).
The time to cross the North Atlantic for a barotropic wave is typically about one week. So, much fast than a baroclinic wave.
The shallow water equations are:
\(u_t-fv=-g\eta_x\\ v_t+fu=-g\eta_y\\ \eta_t+H(u_x+v_y)=0\)
The short wave limit is equivalent to negelcting the \(\eta_t\) term in the continuity equation.
This enables us to work with a streamfunction for which: \(u=-\psi_y,\;v=\psi_x\):
\(\frac{\partial }{\partial t}(\nabla ^2\psi )+\beta\psi_x=0\)
The horizontal divergence is zero. This means that the dvergence flow caused by \(\beta\) must be absorbed by the convergence of the isallobaric flow arising from the \(u_t,\;v_t\)terms.
Note that the isallobaric part of the ageostrophic flow flows towards the isallobaric low, where pressure drops most rapidly. The only way the resulting convergence can be absorbed by the \(\beta\) part is when the waves propagate westward! (is unclear for me)
Explain the concept of normal modes!
The gorverning equations and boundary conditions from a Sturm-Liouville problem so that there is a complete set of (orthogonal) vertical structure functions \(\widehat{p}_n(z),\;\widehat{w}_n(z)\) called vertical normal modes, enabling us to write:
\(u(x,y,z,t)=\sum^\infty_{n=0}\tilde{u_n}(x,y,t)\widehat{p}_n(z)\)
the horizontal structure associated with each mode satisfies the shallow water equations!
\(c_n\)ist the wave speed associated with the n'th mode and \(H_n\) is the equivalent depth.
\(c_0>c_1>c_2>...\)
n=0 is called the barotropic mode. For this mode, \(c=\sqrt{gH}\) (H is the total depth), \(\widehat{p}_0(z)=1\) and \(\widehat{w}_0(z)=\frac{z+H}{H}\) are a good approximation. for the barotropic mode, the vertical velocity varies essentially linearly with depth from zero at the bottom to a maximum at the top and, to good appr., the barotropic velocities \(\tilde{u_0}\) and \(\tilde{v_0}\) are the vertically averaged horizontal velocities.
For \(n\geq1\)we have the baroclinic modes; typically \(c_1=1-3ms^{-1}\)(the first baroclinic mode). For these modes the rigid-lid approximation can be applied, i.e. we can put \(\widehat{w}_n(0)=0\) (i.e. w=0 at Z=0) to a good approximation and all displacements are internal. For the baroclinic modes \(\int^0_{-H}udz=0\) (to a good approximation) and all displacements are internal. For the first mode, \(\widehat{p}_1(z)\) has one zero crossing, for the n'th mode \(\widehat{p}_n(z)\) has n zero crossings.
Note that all modes are "orthogonal", with the implication that each mode varies independently of the others.
the shallow water equations can be obtained from the 3-D governing equations by projecting the 3-D governing equations on to each vertical mode.