# Latent heat benchmark

# Latent heat benchmark#

*This section was contributed by Juliane Dannberg.*

The setup of this benchmark is taken from Schubert, Turcotte and Olson (Schubert, Turcotte, and Olson 2001) (part 1, p. 194) and is illustrated in Fig. 2.

It tests whether the latent heat production when material crosses a phase transition is calculated correctly according to the laws of thermodynamics. The material model defines two phases in the model domain with the phase transition approximately in the center. The material flows in from the top due to a prescribed downward velocity, and crosses the phase transition before it leaves the model domain at the bottom. As initial condition, the model uses a uniform temperature field, however, upon the phase change, latent heat is released. This leads to a characteristic temperature profile across the phase transition with a higher temperature in the bottom half of the domain. To compute it, we have to solve equation [eq:temperature] or its reformulation [eq:temperature-reformulated]. For steady-state one-dimensional downward flow with vertical velocity \(v_y\), it simplifies to the following: $$\begin{gathered} \rho C_p v_y \frac{\partial T}{\partial y} = \rho T \Delta S v_y \frac{\partial X}{\partial y}

\rho C_p \kappa \frac{\partial^2 T}{\partial y^2}.\end{gathered}$\( Here, \)\rho C_p \kappa = k\( with \)k\( the thermal conductivity and \)\kappa\( the thermal diffusivity. The first term on the right-hand side of the equation describes the latent heat produced at the phase transition: It is proportional to the temperature T, the entropy change \)\Delta S\( across the phase transition divided by the specific heat capacity and the derivative of the phase function X. If the velocity is smaller than a critical value, and under the assumption of a discontinuous phase transition (i.e. with a step function as phase function), this latent heating term will be zero everywhere except for the one point \)y_{tr}\( where the phase transition takes place. This means, we have a region above the phase transition with only phase 1, and below a certain depth a jump to a region with only phase 2. Inside of these one-phase regions, we can solve the equation above (using the boundary conditions \)T=T_1\( for \)y \rightarrow \infty\( and \)T=T_2\( for \)y \rightarrow -\infty\() and get \)\(\begin{aligned} T(y) =\begin{cases} T_1 + (T_2-T_1) e^{\frac{v_y (y-y_{tr})}{\kappa}}, & y>y_{tr}\\ T_2, & y<y_{tr} \end{cases}\end{aligned}\)\( While it is not entirely obvious while this equation for \)T(y)\( should be correct (in particular why it should be asymmetric), it is not difficult to verify that it indeed satisfies the equation stated above for both \)y<y_{tr}\( and \)y>y_{tr}\(. Furthermore, it indeed satisfies the jump condition we get by evaluating the equation at \)y=y_{tr}$. Indeed, the jump condition can be reinterpreted as a balance of heat conduction: We know the amount of heat that is produced at the phase boundary, and as we consider only steady-state, the same amount of heat is conducted upwards from the transition:

In contrast to (Schubert, Turcotte, and Olson 2001), we also consider the density change \(\Delta\rho\) across the phase transition: While the heat conduction takes place above the transition and the density can be assumed as \(\rho=\rho_0=\) const., the latent heat is released directly at the phase transition. Thus, we assume an average density \(\rho=\rho_0 + 0.5\Delta\rho\) for the left side of the equation. Rearranging this equation gives

In addition, we have tested the approach exactly as it is described in (Schubert, Turcotte, and Olson 2001) by setting the entropy change to a specific value and in spite of that using a constant density. However, this is physically inconsistent, as the entropy change is proportional to the density change across the phase transition. With this method, we could reproduce the analytic results from (Schubert, Turcotte, and Olson 2001).

The exact values of the parameters used for this benchmark can be found in Fig. 2. They result in a predicted value of \(T_2 = 1109.08 \, \si{K}\) for the temperature in the bottom half of the model, and we will demonstrate below that we can match this value in our numerical computations. However, it is not as simple as suggested above. In actual numerical computations, we can not exactly reproduce the behavior of Dirac delta functions as would result from taking the derivative \(\frac{\partial X}{\partial y}\) of a discontinuous function \(X(y)\). Rather, we have to model \(X(y)\) as a function that has a smooth transition from one value to another, over a depth region of a certain width. In the material model plugin we will use below, this depth is an input parameter and we will play with it in the numerical results shown after the input file.

To run this benchmark, we need to set up an input file that describes the situation. In principle, what we need to do is to describe the position and entropy change of the phase transition in addition to the previously outlined boundary and initial conditions. For this purpose, we use the “latent heat” material model that allows us to set the density change \(\Delta\rho\) and Clapeyron slope \(\gamma\) (which together determine the entropy change via \(\Delta S = \gamma \frac{\Delta\rho}{\rho^2}\)) as well as the depth of the phase transition as input parameters.

All of this setup is then described by the input file cookbooks/latent-heat/latent-heat.prm that models flow in a box of \(10^6\) meters of height and width, and a fixed downward velocity. The following section shows the central part of this file:

```
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The complete input file referenced above also sets the number of mesh refinement steps. For your first runs you will probably want to reduce the number of mesh refinement steps to make things run more quickly. Later on, you might also want to change the phase transition width to look how this influences the result.

Using this input file, let us try to evaluate the results of the current computations. We note that it takes some time for the model to reach a steady state and only then does the bottom temperature reach the theoretical value. Therefore, we use the last output step to compare predicted and computed values. You can visualize the output in different ways, one of it being ParaView and shown in Fig. 2 on the right side (an alternative is to use Visit as described in Section sec:viz). In ParaView, you can plot the temperature profile using the filter “Plot Over Line” (Point1: 500000,0,0; Point2: 500000,1000000,0, then go to the “Display” tab and select “T” as only variable in the “Line series” section) or “Calculator” (as seen in Fig. 2). In Fig. 4 (left) we can see that with increasing resolution, the value for the bottom temperature converges to a value of \(T_2 = 1105.27 \, \si{K}\).

However, this is not what the analytic solution predicted. The reason for this difference is the width of the phase transition with which we smooth out the Dirac delta function that results from differentiating the \(X(y)\) we would have liked to use in an ideal world. (In reality, however, for the Earth’s mantle we also expect phase transitions that are distributed over a certain depth range and so the smoothed out approach may not be a bad approximation.) Of course, the results shown above result from an the analytical approach that is only correct if the phase transition is discontinuous and constrained to one specific depth \(y=y_{tr}\). Instead, we chose a hyperbolic tangent as our phase function. Moreover, Fig. 4 (right) illustrates what happens to the temperature at the bottom when we vary the width of the phase transition: The smaller the width, the closer the temperature gets to the predicted value of \(T_2 = 1109.08 \, \si{K}\), demonstrating that we converge to the correct solution.

Schubert, G., D. L. Turcotte, and P. Olson. 2001. *Mantle Convection in the
Earth and Planets, Part 1*. Cambridge.