Derivation of the Navier–Stokes equations

The derivation of the Navier–Stokes equations as well as their application and formulation for different families of fluids, is an important exercise in fluid dynamics with applications in mechanical engineering, physics, chemistry, heat transfer, and electrical engineering. A proof explaining the properties and bounds of the equations, such as Navier–Stokes existence and smoothness, is one of the important unsolved problems in mathematics.

Basic assumptions

The Navier–Stokes equations are based on the assumption that the fluid, at the scale of interest, is a continuum – a continuous substance rather than discrete particles. Another necessary assumption is that all the fields of interest including pressure, flow velocity, density, and temperature are at least weakly differentiable.

The equations are derived from the basic principles of continuity of mass, conservation of momentum, and conservation of energy. Sometimes it is necessary to consider a finite arbitrary volume, called a control volume, over which these principles can be applied. This finite volume is denoted by Template:Math and its bounding surface Template:Math. The control volume can remain fixed in space or can move with the fluid.

The material derivative

Template:Main Changes in properties of a moving fluid can be measured in two different ways. One can measure a given property by either carrying out the measurement on a fixed point in space as particles of the fluid pass by, or by following a parcel of fluid along its streamline. The derivative of a field with respect to a fixed position in space is called the Eulerian derivative, while the derivative following a moving parcel is called the advective or material (or Lagrangian) derivative.

The material derivative is defined as the linear operator:

$\frac{D}{Dt}\stackrel{\mathrm{d}\mathrm{e}\mathrm{f}}{=}\frac{\partial }{\partial t}+𝐮\cdot \mathrm{\nabla }$

where Template:Math is the flow velocity. The first term on the right-hand side of the equation is the ordinary Eulerian derivative (the derivative on a fixed reference frame, representing changes at a point with respect to time) whereas the second term represents changes of a quantity with respect to position (see advection). This "special" derivative is in fact the ordinary derivative of a function of many variables along a path following the fluid motion; it may be derived through application of the chain rule in which all independent variables are checked for change along the path (which is to say, the total derivative).

For example, the measurement of changes in wind velocity in the atmosphere can be obtained with the help of an anemometer in a weather station or by observing the movement of a weather balloon. The anemometer in the first case is measuring the velocity of all the moving particles passing through a fixed point in space, whereas in the second case the instrument is measuring changes in velocity as it moves with the flow.

Continuity equations

The Navier–Stokes equation is a special continuity equation. A continuity equation may be derived from conservation principles of:

• mass,
• momentum,
• energy.

A continuity equation (or conservation law) is an integral relation stating that the rate of change of some integrated property Template:Mvar defined over a control volume Template:Math must be equal to the rate at which it is lost or gained through the boundaries Template:Math of the volume plus the rate at which it is created or consumed by sources and sinks inside the volume. This is expressed by the following integral continuity equation:

$\frac{d}{dt}\underset{\mathrm{\Omega }}{\int }\phi d\mathrm{\Omega }=-\underset{\mathrm{\Gamma }}{\int }\phi 𝐮\mathbf{\cdot }𝐧d\mathrm{\Gamma }-\underset{\mathrm{\Omega }}{\int }sd\mathrm{\Omega }$

where Template:Math is the flow velocity of the fluid, Template:Math is the outward-pointing unit normal vector, and Template:Mvar represents the sources and sinks in the flow, taking the sinks as positive.

The divergence theorem may be applied to the surface integral, changing it into a volume integral:

$\frac{d}{dt}\underset{\mathrm{\Omega }}{\int }\phi d\mathrm{\Omega }=-\underset{\mathrm{\Omega }}{\int }\mathrm{\nabla }\cdot (\phi 𝐮)d\mathrm{\Omega }-\underset{\mathrm{\Omega }}{\int }sd\mathrm{\Omega }.$

Applying the Reynolds transport theorem to the integral on the left and then combining all of the integrals:

$\underset{\mathrm{\Omega }}{\int }\frac{\partial \phi }{\partial t}d\mathrm{\Omega }=-\underset{\mathrm{\Omega }}{\int }\mathrm{\nabla }\cdot (\phi 𝐮)d\mathrm{\Omega }-\underset{\mathrm{\Omega }}{\int }sd\mathrm{\Omega }\Rightarrow \underset{\mathrm{\Omega }}{\int }(\frac{\partial \phi }{\partial t}+\mathrm{\nabla }\cdot (\phi 𝐮)+s)d\mathrm{\Omega }=0.$

The integral must be zero for any control volume; this can only be true if the integrand itself is zero, so that:

$\frac{\partial \phi }{\partial t}+\mathrm{\nabla }\cdot (\phi 𝐮)+s=0.$

From this valuable relation (a very generic continuity equation), three important concepts may be concisely written: conservation of mass, conservation of momentum, and conservation of energy. Validity is retained if Template:Mvar is a vector, in which case the vector-vector product in the second term will be a dyad.

Conservation of mass

Mass may be considered also. When the intensive property Template:Mvar is considered as the mass, by substitution into the general continuity equation, and taking Template:Math (no sources or sinks of mass):

$\frac{\partial \rho }{\partial t}+\mathrm{\nabla }\cdot (\rho 𝐮)=0$

where Template:Mvar is the mass density (mass per unit volume), and Template:Math is the flow velocity. This equation is called the mass continuity equation, or simply the continuity equation. This equation generally accompanies the Navier–Stokes equation.

In the case of an incompressible fluid, Template:Math (the density following the path of a fluid element is constant) and the equation reduces to:

$\mathrm{\nabla }\cdot 𝐮=0$

which is in fact a statement of the conservation of volume.

Conservation of momentum

A general momentum equation is obtained when the conservation relation is applied to momentum. When the intensive property Template:Mvar is considered as the mass flux (also momentum density), that is, the product of mass density and flow velocity Template:Math, by substitution into the general continuity equation:

$\frac{\partial }{\partial t}(\rho 𝐮)+\mathrm{\nabla }\cdot (\rho 𝐮\otimes 𝐮)=𝐬$

where Template:Math is a dyad, a special case of tensor product, which results in a second rank tensor; the divergence of a second rank tensor is again a vector (a first-rank tensor).

Using the formula for the divergence of a dyad,

$\mathrm{\nabla }\cdot (𝐚\otimes 𝐛)=(\mathrm{\nabla }\cdot 𝐚)𝐛+𝐚\cdot \mathrm{\nabla }𝐛$

we then have

$𝐮\frac{\partial \rho }{\partial t}+\rho \frac{\partial 𝐮}{\partial t}+𝐮\mathrm{\nabla }\cdot (\rho 𝐮)+\rho 𝐮\cdot \mathrm{\nabla }𝐮=𝐬$

Note that the gradient of a vector is a special case of the covariant derivative, the operation results in second rank tensors; except in Cartesian coordinates, it is important to understand that this is not simply an element by element gradient. Rearranging :

$𝐮(\frac{\partial \rho }{\partial t}+\mathrm{\nabla }\cdot (\rho 𝐮))+\rho (\frac{\partial 𝐮}{\partial t}+𝐮\cdot \mathrm{\nabla }𝐮)=𝐬$

The leftmost expression enclosed in parentheses is, by mass continuity (shown before), equal to zero. Noting that what remains on the left side of the equation is the material derivative of flow velocity:

$\rho \frac{D𝐮}{Dt}=\rho (\frac{\partial 𝐮}{\partial t}+𝐮\cdot \mathrm{\nabla }𝐮)=𝐬$

This appears to simply be an expression of Newton's second law (Template:Math) in terms of body forces instead of point forces. Each term in any case of the Navier–Stokes equations is a body force. A shorter though less rigorous way to arrive at this result would be the application of the chain rule to acceleration:

$\begin{array}{cccc}\rho \frac{d}{dt}(𝐮(x,y,z,t))=𝐬& \Rightarrow & \rho (\frac{\partial 𝐮}{\partial t}+\frac{\partial 𝐮}{\partial x}\frac{dx}{dt}+\frac{\partial 𝐮}{\partial y}\frac{dy}{dt}+\frac{\partial 𝐮}{\partial z}\frac{dz}{dt})& =𝐬\\ & \Rightarrow & \rho (\frac{\partial 𝐮}{\partial t}+u\frac{\partial 𝐮}{\partial x}+v\frac{\partial 𝐮}{\partial y}+w\frac{\partial 𝐮}{\partial z})& =𝐬\\ & \Rightarrow & \rho (\frac{\partial 𝐮}{\partial t}+𝐮\cdot \mathrm{\nabla }𝐮)& =𝐬\end{array}$

where Template:Math. The reason why this is "less rigorous" is that we haven't shown that the choice of

$𝐮=(\frac{dx}{dt},\frac{dy}{dt},\frac{dz}{dt})$

is correct; however it does make sense since with that choice of path the derivative is "following" a fluid "particle", and in order for Newton's second law to work, forces must be summed following a particle. For this reason the convective derivative is also known as the particle derivative.

Cauchy momentum equation

Template:See also The generic density of the momentum source Template:Math seen previously is made specific first by breaking it up into two new terms, one to describe internal stresses and one for external forces, such as gravity. By examining the forces acting on a small cube in a fluid, it may be shown that

$\rho \frac{D𝐮}{Dt}=\mathrm{\nabla }\cdot \mathit{\sigma }+\mathit{\rho }f$

where Template:Math is the Cauchy stress tensor, and Template:Math accounts for body forces present. This equation is called the Cauchy momentum equation and describes the non-relativistic momentum conservation of any continuum that conserves mass. Template:Math is a rank two symmetric tensor given by its covariant components. In orthogonal coordinates in three dimensions it is represented as the 3 × 3 matrix:

${\sigma }_{ij}=\left(\begin{array}{ccc}{\sigma }_{xx}& {\tau }_{xy}& {\tau }_{xz}\\ {\tau }_{yx}& {\sigma }_{yy}& {\tau }_{yz}\\ {\tau }_{zx}& {\tau }_{zy}& {\sigma }_{zz}\end{array}\right)$

where the Template:Mvar are normal stresses and Template:Math shear stresses. This matrix is split up into two terms:

${\sigma }_{ij}=\left(\begin{array}{ccc}{\sigma }_{xx}& {\tau }_{xy}& {\tau }_{xz}\\ {\tau }_{yx}& {\sigma }_{yy}& {\tau }_{yz}\\ {\tau }_{zx}& {\tau }_{zy}& {\sigma }_{zz}\end{array}\right)=-\left(\begin{array}{ccc}p& 0& 0\\ 0& p& 0\\ 0& 0& p\end{array}\right)+\left(\begin{array}{ccc}{\sigma }_{xx}+p& {\tau }_{xy}& {\tau }_{xz}\\ {\tau }_{yx}& {\sigma }_{yy}+p& {\tau }_{yz}\\ {\tau }_{zx}& {\tau }_{zy}& {\sigma }_{zz}+p\end{array}\right)=-p𝐈+\mathit{\tau }$

where Template:Math is the 3 × 3 identity matrix and Template:Math is the deviatoric stress tensor. Note that the mechanical pressure Template:Mvar is equal to the negative of the mean normal stress:Template:Sfn

$p=-\frac{1}{3}({\sigma }_{xx}+{\sigma }_{yy}+{\sigma }_{zz}).$

The motivation for doing this is that pressure is typically a variable of interest, and also this simplifies application to specific fluid families later on since the rightmost tensor Template:Math in the equation above must be zero for a fluid at rest. Note that Template:Math is traceless. The Cauchy equation may now be written in another more explicit form:

$\rho \frac{D𝐮}{Dt}=-\mathrm{\nabla }p+\mathrm{\nabla }\cdot \mathit{\tau }+\mathit{\rho }f$

This equation is still incomplete. For completion, one must make hypotheses on the forms of Template:Math and Template:Mvar, that is, one needs a constitutive law for the stress tensor which can be obtained for specific fluid families and on the pressure. Some of these hypotheses lead to the Euler equations (fluid dynamics), other ones lead to the Navier–Stokes equations. Additionally, if the flow is assumed compressible an equation of state will be required, which will likely further require a conservation of energy formulation.

Application to different fluids

The general form of the equations of motion is not "ready for use", the stress tensor is still unknown so that more information is needed; this information is normally some knowledge of the viscous behavior of the fluid. For different types of fluid flow this results in specific forms of the Navier–Stokes equations.

Newtonian fluid

Compressible Newtonian fluid

The formulation for Newtonian fluids stems from an observation made by Newton that, for most fluids,

$\tau \propto \frac{\partial u}{\partial y}$

In order to apply this to the Navier–Stokes equations, three assumptions were made by Stokes:

• The stress tensor is a linear function of the strain rate tensor or equivalently the velocity gradient.
• The fluid is isotropic.
• For a fluid at rest, Template:Math must be zero (so that hydrostatic pressure results).

The above list states the classic argument that the shear strain rate tensor (the (symmetric) shear part of the velocity gradient) is a pure shear tensor and does not include any inflow/outflow part (any compression/expansion part). This means that its trace is zero, and this is achieved by subtracting Template:Math in a symmetric way from the diagonal elements of the tensor. The compressional contribution to viscous stress is added as a separate diagonal tensor.

Applying these assumptions will lead to :

$\mathit{\tau }=\mu (\mathrm{\nabla }𝐮+{\left(\mathrm{\nabla }𝐮\right)}^{𝖳})+\lambda (\mathrm{\nabla }\cdot 𝐮)𝐈$

or in tensor form

${\tau }_{ij}=\mu (\frac{\partial u_i}{\partial x_j}+\frac{\partial u_j}{\partial x_i})+{\delta }_{ij}\lambda \frac{\partial u_k}{\partial x_k}$

That is, the deviatoric of the deformation rate tensor is identified to the deviatoric of the stress tensor, up to a factor Template:Mvar.

Template:Math is the Kronecker delta. Template:Mvar and Template:Mvar are proportionality constants associated with the assumption that stress depends on strain linearly; Template:Mvar is called the first coefficient of viscosity or shear viscosity (usually just called "viscosity") and Template:Mvar is the second coefficient of viscosity or volume viscosity (and it is related to bulk viscosity). The value of Template:Mvar, which produces a viscous effect associated with volume change, is very difficult to determine, not even its sign is known with absolute certainty. Even in compressible flows, the term involving Template:Mvar is often negligible; however it can occasionally be important even in nearly incompressible flows and is a matter of controversy. When taken nonzero, the most common approximation is Template:Math.Template:Sfn

A straightforward substitution of Template:Math into the momentum conservation equation will yield the Navier–Stokes equations, describing a compressible Newtonian fluid:

$\rho (\frac{\partial 𝐮}{\partial t}+𝐮\cdot \mathrm{\nabla }𝐮)=-\mathrm{\nabla }p+\mathrm{\nabla }\cdot \left[\mu (\mathrm{\nabla }𝐮+{\left(\mathrm{\nabla }𝐮\right)}^{𝖳})\right]+\mathrm{\nabla }\cdot \left[\lambda (\mathrm{\nabla }\cdot 𝐮)𝐈\right]+\rho 𝐠$

The body force has been decomposed into density and external acceleration, that is, Template:Math. The associated mass continuity equation is:

$\frac{\partial \rho }{\partial t}+\mathrm{\nabla }\cdot (\rho 𝐮)=0$

In addition to this equation, an equation of state and an equation for the conservation of energy is needed. The equation of state to use depends on context (often the ideal gas law), the conservation of energy will read:

$\rho \frac{Dh}{Dt}=\frac{Dp}{Dt}+\mathrm{\nabla }\cdot (k\mathrm{\nabla }T)+\mathrm{\Phi }$

Here, Template:Mvar is the specific enthalpy, Template:Mvar is the temperature, and Template:Math is a function representing the dissipation of energy due to viscous effects:

$\mathrm{\Phi }=\mu (2{\left(\frac{\partial u}{\partial x}\right)}^2+2{\left(\frac{\partial v}{\partial y}\right)}^2+2{\left(\frac{\partial w}{\partial z}\right)}^2+{(\frac{\partial v}{\partial x}+\frac{\partial u}{\partial y})}^2+{(\frac{\partial w}{\partial y}+\frac{\partial v}{\partial z})}^2+{(\frac{\partial u}{\partial z}+\frac{\partial w}{\partial x})}^2)+\lambda (\mathrm{\nabla }\cdot 𝐮{)}^2.$

With a good equation of state and good functions for the dependence of parameters (such as viscosity) on the variables, this system of equations seems to properly model the dynamics of all known gases and most liquids.

Incompressible Newtonian fluid

For the special (but very common) case of incompressible flow, the momentum equations simplify significantly. Using the following assumptions:

• Viscosity Template:Mvar will now be a constant
• The second viscosity effect Template:Math
• The simplified mass continuity equation Template:Math

This gives incompressible Navier-Stokes equations, describing incompressible Newtonian fluid:

$\rho (\frac{\partial 𝐮}{\partial t}+𝐮\cdot \mathrm{\nabla }𝐮)=-\mathrm{\nabla }p+\mathrm{\nabla }\cdot \left[\mu (\mathrm{\nabla }𝐮+{\left(\mathrm{\nabla }𝐮\right)}^{𝖳})\right]+\rho 𝐠$

then looking at the viscous terms of the Template:Mvar momentum equation for example we have:

$\begin{array}{cc}& \frac{\partial }{\partial x}\left(2\mu \frac{\partial u}{\partial x}\right)+\frac{\partial }{\partial y}\left(\mu (\frac{\partial u}{\partial y}+\frac{\partial v}{\partial x})\right)+\frac{\partial }{\partial z}\left(\mu (\frac{\partial u}{\partial z}+\frac{\partial w}{\partial x})\right)\\ [8px]& =2\mu \frac{{\partial }^{2}u}{\partial x^2}+\mu \frac{{\partial }^{2}u}{\partial y^2}+\mu \frac{{\partial }^{2}v}{\partial y\partial x}+\mu \frac{{\partial }^{2}u}{\partial z^2}+\mu \frac{{\partial }^{2}w}{\partial z\partial x}\\ [8px]& =\mu \frac{{\partial }^{2}u}{\partial x^2}+\mu \frac{{\partial }^{2}u}{\partial y^2}+\mu \frac{{\partial }^{2}u}{\partial z^2}+\mu \frac{{\partial }^{2}u}{\partial x^2}+\mu \frac{{\partial }^{2}v}{\partial y\partial x}+\mu \frac{{\partial }^{2}w}{\partial z\partial x}\\ [8px]& =\mu {\mathrm{\nabla }}^{2}u+\mu \frac{\partial }{\partial x}{\xcancel{(\frac{\partial u}{\partial x}+\frac{\partial v}{\partial y}+\frac{\partial w}{\partial z})}}^0\\ [8px]& =\mu {\mathrm{\nabla }}^{2}u\end{array}$

Similarly for the Template:Mvar and Template:Mvar momentum directions we have Template:Math and Template:Math.

The above solution is key to deriving Navier–Stokes equations from the equation of motion in fluid dynamics when density and viscosity are constant.

Non-Newtonian fluids

Template:Main A non-Newtonian fluid is a fluid whose flow properties differ in any way from those of Newtonian fluids. Most commonly the viscosity of non-Newtonian fluids is a function of shear rate or shear rate history. However, there are some non-Newtonian fluids with shear-independent viscosity, that nonetheless exhibit normal stress-differences or other non-Newtonian behaviour. Many salt solutions and molten polymers are non-Newtonian fluids, as are many commonly found substances such as ketchup, custard, toothpaste, starch suspensions, paint, blood, and shampoo. In a Newtonian fluid, the relation between the shear stress and the shear rate is linear, passing through the origin, the constant of proportionality being the coefficient of viscosity. In a non-Newtonian fluid, the relation between the shear stress and the shear rate is different, and can even be time-dependent. The study of the non-Newtonian fluids is usually called rheology. A few examples are given here.

Bingham fluid

In Bingham fluids, the situation is slightly different:

$\frac{\partial u}{\partial y}=\{\begin{array}{cc}0,& \tau <{\tau }_0\\ [5px]\frac{\tau -{\tau }_0}{\mu },& \tau \ge {\tau }_0\end{array}$

These are fluids capable of bearing some stress before they start flowing. Some common examples are toothpaste and clay.

Power-law fluid

A power law fluid is an idealised fluid for which the shear stress, Template:Mvar, is given by

$\tau =K{\left(\frac{\partial u}{\partial y}\right)}^n$

This form is useful for approximating all sorts of general fluids, including shear thinning (such as latex paint) and shear thickening (such as corn starch water mixture).

Stream function formulation

In the analysis of a flow, it is often desirable to reduce the number of equations and/or the number of variables. The incompressible Navier–Stokes equation with mass continuity (four equations in four unknowns) can be reduced to a single equation with a single dependent variable in 2D, or one vector equation in 3D. This is enabled by two vector calculus identities:

$\begin{array}{cc}\mathrm{\nabla }\times (\mathrm{\nabla }\varphi )& =0\\ \mathrm{\nabla }\cdot (\mathrm{\nabla }\times 𝐀)& =0\end{array}$

for any differentiable scalar Template:Mvar and vector Template:Math. The first identity implies that any term in the Navier–Stokes equation that may be represented as the gradient of a scalar will disappear when the curl of the equation is taken. Commonly, pressure Template:Mvar and external acceleration Template:Math will be eliminated, resulting in (this is true in 2D as well as 3D):

$\mathrm{\nabla }\times (\frac{\partial 𝐮}{\partial t}+𝐮\cdot \mathrm{\nabla }𝐮)=\nu \mathrm{\nabla }\times \left({\mathrm{\nabla }}^2𝐮\right)$

where it is assumed that all body forces are describable as gradients (for example it is true for gravity), and density has been divided so that viscosity becomes kinematic viscosity.

The second vector calculus identity above states that the divergence of the curl of a vector field is zero. Since the (incompressible) mass continuity equation specifies the divergence of flow velocity being zero, we can replace the flow velocity with the curl of some vector Template:Math so that mass continuity is always satisfied:

$\mathrm{\nabla }\cdot 𝐮=0\Rightarrow \mathrm{\nabla }\cdot (\mathrm{\nabla }\times \mathit{\psi })=0\Rightarrow 0=0$

So, as long as flow velocity is represented through Template:Math, mass continuity is unconditionally satisfied. With this new dependent vector variable, the Navier–Stokes equation (with curl taken as above) becomes a single fourth order vector equation, no longer containing the unknown pressure variable and no longer dependent on a separate mass continuity equation:

$\mathrm{\nabla }\times (\frac{\partial }{\partial t}(\mathrm{\nabla }\times \mathit{\psi })+(\mathrm{\nabla }\times \mathit{\psi })\cdot \mathrm{\nabla }(\mathrm{\nabla }\times \mathit{\psi }))=\nu \mathrm{\nabla }\times ({\mathrm{\nabla }}^2(\mathrm{\nabla }\times \mathit{\psi }))$

Apart from containing fourth order derivatives, this equation is fairly complicated, and is thus uncommon. Note that if the cross differentiation is left out, the result is a third order vector equation containing an unknown vector field (the gradient of pressure) that may be determined from the same boundary conditions that one would apply to the fourth order equation above.

2D flow in orthogonal coordinates

The true utility of this formulation is seen when the flow is two dimensional in nature and the equation is written in a general orthogonal coordinate system, in other words a system where the basis vectors are orthogonal. Note that this by no means limits application to Cartesian coordinates, in fact most of the common coordinates systems are orthogonal, including familiar ones like cylindrical and obscure ones like toroidal.

The 3D flow velocity is expressed as (note that the discussion not used coordinates so far):

$𝐮=u_1{𝐞}_1+u_2{𝐞}_2+u_3{𝐞}_3$

where Template:Math are basis vectors, not necessarily constant and not necessarily normalized, and Template:Math are flow velocity components; let also the coordinates of space be Template:Math.

Now suppose that the flow is 2D. This does not mean the flow is in a plane, rather it means that the component of flow velocity in one direction is zero and the remaining components are independent of the same direction. In that case (take component 3 to be zero):

$𝐮=u_1{𝐞}_1+u_2{𝐞}_2;\frac{\partial u_1}{\partial x_3}=\frac{\partial u_2}{\partial x_3}=0$

The vector function Template:Math is still defined via:

$𝐮=\mathrm{\nabla }\times \mathit{\psi }$

but this must simplify in some way also since the flow is assumed 2D. If orthogonal coordinates are assumed, the curl takes on a fairly simple form, and the equation above expanded becomes:

$u_1{𝐞}_1+u_2{𝐞}_2=\frac{{𝐞}_1}{h_2{h}_3}[\frac{\partial }{\partial x_2}\left(h_3{\psi }_3\right)-\frac{\partial }{\partial x_3}\left(h_2{\psi }_2\right)]+$

$+\frac{{𝐞}_2}{h_3{h}_1}[\frac{\partial }{\partial x_3}\left(h_1{\psi }_1\right)-\frac{\partial }{\partial x_1}\left(h_3{\psi }_3\right)]+\frac{{𝐞}_3}{h_1{h}_2}[\frac{\partial }{\partial x_1}\left(h_2{\psi }_2\right)-\frac{\partial }{\partial x_2}\left(h_1{\psi }_1\right)]$

Examining this equation shows that we can set Template:Math and retain equality with no loss of generality, so that:

$u_1{𝐞}_1+u_2{𝐞}_2=\frac{{𝐞}_1}{h_2{h}_3}\frac{\partial }{\partial x_2}\left(h_3{\psi }_3\right)-\frac{{𝐞}_2}{h_3{h}_1}\frac{\partial }{\partial x_1}\left(h_3{\psi }_3\right)$

the significance here is that only one component of Template:Math remains, so that 2D flow becomes a problem with only one dependent variable. The cross differentiated Navier–Stokes equation becomes two Template:Math equations and one meaningful equation.

The remaining component Template:Math is called the stream function. The equation for Template:Mvar can simplify since a variety of quantities will now equal zero, for example:

$\mathrm{\nabla }\cdot \mathit{\psi }=\frac{1}{h_1{h}_2{h}_3}\frac{\partial }{\partial x_3}\left(\psi h_1{h}_2\right)=0$

if the scale factors Template:Math and Template:Math also are independent of Template:Math. Also, from the definition of the vector Laplacian

$\mathrm{\nabla }\times (\mathrm{\nabla }\times \mathit{\psi })=\mathrm{\nabla }(\mathrm{\nabla }\cdot \mathit{\psi })-{\mathrm{\nabla }}^2\mathit{\psi }=-{\mathrm{\nabla }}^2\mathit{\psi }$

Manipulating the cross differentiated Navier–Stokes equation using the above two equations and a variety of identities will eventually yield the 1D scalar equation for the stream function:

$\frac{\partial }{\partial t}\left({\mathrm{\nabla }}^2\psi \right)+(\mathrm{\nabla }\times \mathit{\psi })\cdot \mathrm{\nabla }\left({\mathrm{\nabla }}^2\psi \right)=\nu {\mathrm{\nabla }}^4\psi$

where Template:Math is the biharmonic operator. This is very useful because it is a single self-contained scalar equation that describes both momentum and mass conservation in 2D. The only other equations that this partial differential equation needs are initial and boundary conditions.

Derivation of the scalar stream function equation

Distributing the curl: $\frac{\partial }{\partial t}(\mathrm{\nabla }\times (\mathrm{\nabla }\times \mathit{\psi }))+\mathrm{\nabla }\times ((\mathrm{\nabla }\times \mathit{\psi })\cdot \mathrm{\nabla }(\mathrm{\nabla }\times \mathit{\psi }))=\nu \mathrm{\nabla }\times ({\mathrm{\nabla }}^2(\mathrm{\nabla }\times \mathit{\psi }))$ Replacing curl of the curl with the Laplacian and expanding convection and viscosity: $-\frac{\partial }{\partial t}\left({\mathrm{\nabla }}^2\mathit{\psi }\right)+\mathrm{\nabla }\times (\mathrm{\nabla }\left(\frac{(\mathrm{\nabla }\times \mathit{\psi })\cdot (\mathrm{\nabla }\times \mathit{\psi })}{2}\right)+(\mathrm{\nabla }\times (\mathrm{\nabla }\times \mathit{\psi }))\times (\mathrm{\nabla }\times \mathit{\psi }))=\nu ({\mathrm{\nabla }}^2(\mathrm{\nabla }(\mathrm{\nabla }\cdot \mathit{\psi }))-{\mathrm{\nabla }}^4\mathit{\psi })$ Above, the curl of a gradient is zero, and the divergence of Template:Math is zero. Negating: $\frac{\partial }{\partial t}\left({\mathrm{\nabla }}^2\mathit{\psi }\right)+\mathrm{\nabla }\times ({\mathrm{\nabla }}^2\mathit{\psi }\times (\mathrm{\nabla }\times \mathit{\psi }))=\nu {\mathrm{\nabla }}^4\mathit{\psi }$ Expanding the curl of the cross product into four terms: $\frac{\partial }{\partial t}\left({\mathrm{\nabla }}^2\mathit{\psi }\right)+(\mathrm{\nabla }\times \mathit{\psi })\cdot \mathrm{\nabla }\left({\mathrm{\nabla }}^2\mathit{\psi }\right)-\left({\mathrm{\nabla }}^2\mathit{\psi }\right)\cdot \mathrm{\nabla }(\mathrm{\nabla }\times \mathit{\psi })+\left({\mathrm{\nabla }}^2\mathit{\psi }\right)(\mathrm{\nabla }\cdot (\mathrm{\nabla }\times \mathit{\psi }))-(\mathrm{\nabla }\times \mathit{\psi })(\mathrm{\nabla }\cdot \left({\mathrm{\nabla }}^2\mathit{\psi }\right))=\nu {\mathrm{\nabla }}^4\mathit{\psi }$ Only one of four terms of the expanded curl is nonzero. The second is zero because it is the dot product of orthogonal vectors, the third is zero because it contains the divergence of flow velocity, and the fourth is zero because the divergence of a vector with only component three is zero (since it is assumed that nothing (except maybe Template:Math) depends on component three). $\frac{\partial }{\partial t}\left({\mathrm{\nabla }}^2\mathit{\psi }\right)+(\mathrm{\nabla }\times \mathit{\psi })\cdot \mathrm{\nabla }\left({\mathrm{\nabla }}^2\mathit{\psi }\right)=\nu {\mathrm{\nabla }}^4\mathit{\psi }$ This vector equation is one meaningful scalar equation and two Template:Math equations.

The assumptions for the stream function equation are:

• The flow is incompressible and Newtonian.
• Coordinates are orthogonal.
• Flow is 2D: Template:Math
• The first two scale factors of the coordinate system are independent of the last coordinate: Template:Math, otherwise extra terms appear.

The stream function has some useful properties:

• Since Template:Math, the vorticity of the flow is just the negative of the Laplacian of the stream function.
• The level curves of the stream function are streamlines.

The stress tensor

The derivation of the Navier–Stokes equation involves the consideration of forces acting on fluid elements, so that a quantity called the stress tensor appears naturally in the Cauchy momentum equation. Since the divergence of this tensor is taken, it is customary to write out the equation fully simplified, so that the original appearance of the stress tensor is lost.

However, the stress tensor still has some important uses, especially in formulating boundary conditions at fluid interfaces. Recalling that Template:Math, for a Newtonian fluid the stress tensor is:

${\sigma }_{ij}=-p{\delta }_{ij}+\mu (\frac{\partial u_i}{\partial x_j}+\frac{\partial u_j}{\partial x_i})+{\delta }_{ij}\lambda \mathrm{\nabla }\cdot 𝐮.$

If the fluid is assumed to be incompressible, the tensor simplifies significantly. In 3D cartesian coordinates for example:

$\begin{array}{cc}\mathit{\sigma }& =-\left(\begin{array}{ccc}p& 0& 0\\ 0& p& 0\\ 0& 0& p\end{array}\right)+\mu \left(\begin{array}{ccc}2\frac{\partial u}{\partial x}& \frac{\partial u}{\partial y}+\frac{\partial v}{\partial x}& \frac{\partial u}{\partial z}+\frac{\partial w}{\partial x}\\ \frac{\partial v}{\partial x}+\frac{\partial u}{\partial y}& 2\frac{\partial v}{\partial y}& \frac{\partial v}{\partial z}+\frac{\partial w}{\partial y}\\ \frac{\partial w}{\partial x}+\frac{\partial u}{\partial z}& \frac{\partial w}{\partial y}+\frac{\partial v}{\partial z}& 2\frac{\partial w}{\partial z}\end{array}\right)\\ [6px]& =-p𝐈+\mu (\mathrm{\nabla }𝐮+{\left(\mathrm{\nabla }𝐮\right)}^{𝖳})\\ [6px]& =-p𝐈+2\mu 𝐞\end{array}$

Template:Math is the strain rate tensor, by definition:

$e_{ij}=\frac{1}{2}(\frac{\partial u_i}{\partial x_j}+\frac{\partial u_j}{\partial x_i}).$

See also

• Derivation of Navier–Stokes equation from discrete LBE
• First law of thermodynamics (fluid mechanics)

References

• Template:Cite book
• Template:Cite book
• Surface Tension Module Template:Webarchive, by John W. M. Bush, at MIT OCW
• Galdi, An Introduction to the Mathematical Theory of the Navier–Stokes Equations: Steady-State Problems. Springer 2011