3.2.1. Low Mach Number Equations

The low Mach number equations are a subset of the full compressible Navier-Stokes (and continuity and energy) equations, admitting large variations in gas density while remaining acoustically incompressible. The low Mach number equations are preferred over the full compressible equations for our problems of interest. We avoid resolving fast-moving acoustic signals which have no bearing on the transport processes. Derivations of the low Mach number equations are found in Rehm and Baum [2], Paolucci [3], Majda and Sethian [4], and Merkle and Choi [5]. The equations are derived from the compressible equations using a perturbation expansion in terms of the lower limit of the Mach number squared; hence the name. The asymptotic expansion leads to a splitting of pressure into a spatially constant thermodynamic pressure and a locally varying dynamic pressure. The dynamic pressure is decoupled from the thermodynamic state and cannot propagate acoustic waves. The thermodynamic pressure is used in the equation of state and to determine thermophysical properties. The thermodynamic pressure can vary in time and can be calculated using a global energy balance.

3.2.1.1. Asymptotic Expansion

The asymptotic expansion for the low Mach number equations begins with the full compressible equations in Cartesian coordinates. The equations are the minimum set required to propagate acoustic waves. The equations are written in divergence form using Einstein notation (summation over repeated indices):

(3.1) ${{\partial \rho} \over {\partial t}} + {{\partial \rho u_j} \over {\partial x_j}} = 0 ,$

(3.2) ${{\partial \rho u_i} \over {\partial t}} + {{\partial \rho u_j u_i} \over {\partial x_j}} + {{\partial P} \over {\partial x_i}} = {{\partial \tau_{ij}} \over {\partial x_j}} + \rho g_i ,$

(3.3) ${{\partial \rho E} \over {\partial t}} + {{\partial \rho u_j H} \over {\partial x_j}} = - {{\partial q_j} \over {\partial x_j}} + {{\partial u_i \tau_{ij}} \over {\partial x_j}} + \rho u_i g_i .$

The primitive variables are the velocity components, $u_i$ , the pressure, $P$ , and the temperature $T$ . The viscous shear stress tensor is $\tau_{ij}$ , the heat conduction is $q_i$ , the total enthalpy is $H$ , the total internal energy is $E$ , the density is $\rho$ , and the gravity vector is $g_i$ . The total internal energy and total enthalpy contain the kinetic energy contributions. The equations are closed using the following models and definitions:

(3.4) $P = \rho {R \over W} T ,$

(3.5) $E = H - P/\rho ,$

(3.6) $H = h + {1 \over 2} u_k u_k ,$

(3.7) $\tau_{ij} = \mu \left( {{\partial u_i} \over {\partial x_j}} + {{\partial u_j} \over {\partial x_i}} \right) - {2 \over 3} \mu {{\partial u_k} \over {\partial x_k}} \delta_{ij} ,$

(3.8) $q_i = - k {{\partial T} \over {\partial x_i}} .$

The mean molecular weight of the gas is $W$ , the molecular viscosity is $\mu$ , and the thermal conductivity is $k$ . A Newtonian fluid is assumed along with the Stokes hypothesis for the stress tensor.

The equations are scaled so that the variables are all of order one. The velocities, lengths, and times are nondimensionalized by a characteristic velocity, $U_\infty$ , and a length scale, $L$ . The pressure, density, and temperature are nondimensionalized by $P_\infty$ , $\rho_\infty$ , and $T_\infty$ . The enthalpy and energy are nondimensionalized by $C_{p,\infty} T_\infty$ . Dimensionless variables are noted by overbars. The dimensionless equations are:

(3.9) ${{\partial \bar{\rho}} \over {\partial \bar{t}}} + {{\partial \bar{\rho} \bar{u}_j}\over {\partial \bar{x}_j}} = 0 ,$

(3.10) ${{\partial \bar{\rho} \bar{u}_i} \over {\partial \bar{t}}} + {{\partial \bar{\rho} \bar{u}_j \bar{u}_i} \over {\partial \bar{x}_j}} + {1 \over {\gamma {\rm Ma}^2}} {{\partial \bar{P}} \over {\partial \bar{x}_i}} = {1 \over {\rm Re}}{{\partial \bar{\tau}_{ij}} \over {\partial \bar{x}_j}} + {1 \over {\rm Fr}_i} \bar{\rho} {{\partial \bar{\rho} \bar{h}} \over {\partial \bar{t}}} + {{\partial \bar{\rho} \bar{u}_j \bar{h}} \over {\partial \bar{x}_j}} = - {1 \over {\rm Pr}} {1 \over {\rm Re}} {{\partial \bar{q}_j} \over {\partial \bar{x}_j}} + {{\gamma - 1} \over \gamma} {{\partial \bar{P}} \over {\partial \bar{t}}} + {{\gamma - 1} \over \gamma} {{{\rm Ma}^2} \over {\rm Re}} {{\partial \bar{u}_i \bar{\tau}_{ij}} \over {\partial \bar{x}_j}} + \bar{\rho} \bar{u}_i {{\gamma - 1} \over \gamma} {{{\rm Ma}^2} \over {\rm Fr}_i}$

$- {{\gamma - 1} \over 2} {\rm Ma}^2 \left( {{\partial \bar{\rho} \bar{u}_k \bar{u}_k} \over {\partial \bar{t}}} + {{\partial \bar{\rho} \bar{u}_j \bar{u}_k \bar{u}_k} \over {\partial \bar{x}_j}} \right) .$

The groupings of characteristic scaling terms are:

(3.11) ${\rm Re} = {{\rho_\infty U_\infty L} \over {\mu_\infty}}, \quad \quad \phantom{xxx} \mbox{\rm Reynolds number},$

(3.12) ${\rm Pr} = {{C_{p,\infty} \mu_\infty} \over {k_\infty}}, \quad \quad \phantom{xxx} \mbox{\rm Prandtl number},$

(3.13) ${\rm Fr}_i = {{u_\infty^2} \over {g_i L}}, \quad \quad \phantom{xxxxxxi} \mbox{\rm Froude number}, \quad g_i \ne 0,$

(3.14) ${\rm Ma} = \sqrt{{u^2_\infty} \over {\gamma R T_\infty /W}}, \quad \quad \mbox{\rm Mach number},$

where $\gamma$ is the ratio of specific heats.

For small Mach numbers, ${\rm Ma} \ll 1$ , the kinetic energy, viscous work, and gravity work terms can be neglected in the energy equation since those terms are scaled by the square of the Mach number. The inverse of Mach number squared remains in the momentum equations, suggesting singular behavior. In order to explore the singularity, the pressure, velocity and temperature are expanded as asymptotic series in terms of the parameter $\epsilon$ :

(3.15) $\bar{P} = \bar{P}_0 + \bar{P}_1 \epsilon + \bar{P}_2 \epsilon^2 \ldots$

(3.16) $\bar{u}_i = \bar{u}_{i,0} + \bar{u}_{i,1} \epsilon + \bar{u}_{i,2} \epsilon^2 \ldots$

(3.17) $\bar{T} = \bar{T}_0 + \bar{T}_1 \epsilon + \bar{T}_2 \epsilon^2 \ldots$

The zeroth-order terms are collected together in each of the equations. The form of the continuity equation stays the same. The gradient of the pressure in the zeroth-order momentum equations can become singular since it is divided by the characteristic Mach number squared. In order for the zeroth-order momentum equations to remain well-behaved, the spatial variation of the $\bar{P}_0$ term must be zero. If the magnitude of the expansion parameter is selected to be proportional to the square of the characteristic Mach number, $\epsilon = \gamma {\rm Ma}^2$ , then the $\bar{P}_1$ term can be included in the zeroth-order momentum equation.

(3.18) ${1 \over {\gamma {\rm Ma}^2}} {{\partial \bar{P}} \over {\partial x_i}} = {{\partial} \over {\partial x_i}} \left( {1 \over {\gamma {\rm Ma}^2}} \bar{P}_0 + {\epsilon \over {\gamma {\rm Ma}^2}} \bar{P}_1 + \ldots \right) = {{\partial} \over {\partial x_i}} \left( \bar{P}_1 + \epsilon \bar{P}_2 + \ldots \phantom{1 \over {\gamma {\rm Ma}^2}} \right)$

The form of the energy equation remains the same, less the kinetic energy, viscous work and gravity work terms. The $P_0$ term remains in the energy equation as a time derivative. The low Mach number equations are the zeroth-order equations in the expansion including the $P_1$ term in the momentum equations. The expansion results in two different types of pressure and they are considered to be split into a thermodynamic component and a dynamic component. The thermodynamic pressure is constant in space, but can change in time. The thermodynamic pressure is used in the equation of state. The dynamic pressure only arises as a gradient term in the momentum equation and acts to enforce continuity. The un-split dimensional pressure is

(3.19) $P = P_{th} + \gamma {\rm Ma}^2 P_1,$

where the dynamic pressure, $p=P-P_{th}$ , is related to a pressure coefficient

(3.20) $\bar{P}_1 = {{P - P_{th}} \over {\rho_\infty u^2_\infty}} P_{th}.$

The resulting unscaled low Mach number equations are:

(3.21) ${{\partial \rho} \over {\partial t}} + {{\partial \rho u_j} \over {\partial x_j}} = 0,$

(3.22) ${{\partial \rho u_i} \over {\partial t}} + {{\partial \rho u_j u_i} \over {\partial x_j}} + {{\partial p} \over {\partial x_i}} = {{\partial \tau_{ij}} \over {\partial x_j}} + \left( \rho - \rho_{\circ} \right) g_i,$

(3.23) ${{\partial \rho h} \over {\partial t}} + {{\partial \rho u_j h} \over {\partial x_j}} = - {{\partial q_j} \over {\partial x_j}} + {{\partial P_{th}} \over {\partial t}},$

where the ideal gas law becomes

(3.24) $P_{th} = \rho {R \over W} T.$

The hydrostatic pressure gradient has been subtracted from the momentum equation, assuming an ambient density of $\rho_{\circ}$ . The stress tensor and heat conduction remain the same as in the original equations.

3.2.1.2. Variable Thermodynamic Pressure

For a low Mach number set of equations, the time derivative of pressure can only be nonzero in a closed volume with energy addition or subtraction. Relaxing the low Mach number limit allows a time and spatially varying pressure to appear in the energy equation (see Conservation of Energy).