Open access peer-reviewed chapter

Fluid Motion Equations in Tensor Form

By Dmitry Nikushchenko and Valery Pavlovsky

Submitted: November 20th 2019Reviewed: January 21st 2020Published: March 11th 2020

DOI: 10.5772/intechopen.91284

Downloaded: 83

Abstract

In the current chapter, some applications of tensor analysis to fluid dynamics are presented. Governing equations of fluid motion and energy are obtained and analyzed. We shall discuss about continuity equation, equation of motion, and mechanical energy transport equation and four forms of energy equation. Finally, we shall talk about the divergence from transfer equations of different parameters of motion. The tensor form of equations has advantages over the component form: these are, first, compact writing of equations and, second, independency from reference frames, etc. Moreover, it allows to obtain new forms of equations on the basis of governing ones easily.

Keywords

  • stress tensor
  • Navier–stokes equation
  • energy
  • continuity
  • vorticity
  • divergence form

1. Introduction

The mathematical model of moving fluid includes a set of equations, which are usually written as transport equations of main physical parameters—density, velocity, energy, etc. These equations are conservation laws in fluid flows. Traditionally the component form of the equations is usually used, but at the same time, the componentless form (Gibbs approach) could be applied to obtain and transform these equations. In this chapter several main conservation laws are discussed and represented in tensor form, which has many advantages against usually used component form, like simplicity and compactness, independence on reference frames, less errors in transformations, etc. Below we obtain and analyze continuity and momentum equations and vorticity and energy transport equations, and we discuss also about the divergent form of transport Eqs.

2. Continuity equation

Continuity equation is the mass conservation law for a fluid flow and is presented as a scalar equation, which connects density ρ and velocity of fluid particles V, and for any liquid it could be written as

ρt+Vρ+ρV=0,E1

where =eixi=e1x1+e2x2+e2x3is the Hamilton operator and the dot is a symbol of a scalar product.

Hereinafter, the Einstein summation convention is used by default.

It also can be written in two other equivalent forms [1, 2]:

dρdt+ρV=0andρt+ρV=0.E2

In the case of incompressible fluid, we could obtain its simplified form:

V=0.E3

Let us apply gradient operator to continuity equation (Eq. (1)):

ρt+Vρ+ρV=0.

As a result, we obtain vector equation:

tρ+ρVT+Vρ+Vρ+ρV=0,E4

which could be written in a more compact form:

ddtρ+Vρ+Vρ+ρV=0E5

or by a little bit different way:

ddtρ+Vρ+ρV=0.E6

These equations contain gradient of vector Vdivergence, which [3] equal to

V=ΔV+××V.

For incompressible fluid the left part of this relation is equal to zero; therefore for rotation of velocity vector, we can write:

××V=ΔV.E7

In the case of compressible fluid in accordance with Eq. (6), we have additional terms in the right part of the equation:

××V=ΔV+1ρddtρ+1ρVρ+Vρρ.E8

Continuity equation can be also written in tensor form:

13trρtE¯+trρV=0.E9

The tensor ρVcan be represented as

ρV=ekxkρVjej=xkρVjekej==ρxkVj+ρVjxkekej=ρV+ρV.E10

Finally, continuity equation can be written in form

ρt+trρV+ρV=0.E11

Convective derivatives of density and pressure (and any another scalar quantitatives) also can be written in tensor form:

Vρ=trVρ;Vp=trVp,

i.e., convective derivative is equal to trace of corresponding tensor.

In addition, for the divergence of the product of scalar and vector functions, we can obtain the following relation:

ρV=ρV+ρV:E¯.

3. Equations of motion of fluid with constant and variable properties

The equation of a motion in terms of stress [4, 5] is

ρdVdt=σ¯+ρf,E12

where fis the body force per unit mass and σ¯is the divergence of stress tensor σ¯. In accordance with Newton’s law, tensor σ¯for an incompressible fluid is

σ¯=pE¯+2μS¯,E13

where p is the pressure; μ is the fluid shear (dynamic) viscosity; and S¯=12V+VTis the rate of strain tensor. Due to relation V=0, when μconstdivergence of stress tensor σ¯is written as

σ¯=p+μ2S¯+2μS¯=p+μ2S¯+μΔV.E14

Then equation of motion of incompressible fluid (Navier–Stokes equation) at μconstis

ρdVdt=p+μΔV+μ2S¯+ρf.E15

Additional term μ2S¯relates to changing of shear viscosity. In Cartesian coordinates Eq. (15) has the form:

ρdVidt=pxi+μΔVi+μxjVjxi+Vixj+ρfi.

In case of compressible fluid with variable viscosity, the equation will contain a term with divergence V,which is not equal to zero now. Rheological relation is this case has the form [2]:

σ¯=pE¯23μVE¯+2μS¯.E16

Let us introduce the denotation:

p+23μV=p;E17

then we can write Eq. (16) as

σ¯=pE¯+2μS¯.E18

Divergence of this tensor at μconstis

σ¯=p+μ2S¯+μΔV+μV.

As a result, equation of motion of compressible fluid with variable viscosity has the form:

ρdVdt=p+μΔV+μV+μ2S¯+ρf,E19

in Cartesian coordinates

ρVit+VjVixj=pxi+μΔVi+μxiVjxj+μxjVjxi+Vixj+ρfi.

If we represent fluid particle acceleration as the sum of local and convective terms, then (Eq. (19)) will take the form:

ρVt+ρVV=p+μΔV+μV+μ2S¯+ρf,E20

considering viscosity variability is especially important for turbulent flow modeling using the Boussinesq hypothesis with turbulent viscosity μt.

Let us apply divergence operation to the Navier–Stokes equation for compressible fluid with variable viscosity. With this purpose we shall apply operation to each vector term of Eq. (20):

ρVt=ρVt+ρtV;ρVV=ρVV+ρV:V+ρVV;p=Δp;μΔV=μΔV+μΔV;μV=μV+μΔV;μ2S¯=μ:V+μV+μ:VT+μΔV.

If the fluid motion occurs in gravity force field, then there is potential U=gz, where z is the vertical coordinate and the body force per unit mass is f=U. In this case ρf=ρf+ρf=ρUρΔU.

Function U is linear; therefore ΔU=0and

ρf=ρU.

As a result of applied divergence operation to Navier–Stokes equation at μconst, we obtain scalar equation:

ρddtV+ρdVdt+ρV:V=Δp'+2μΔV+V++2μΔV+:2μS¯ρU.E21

In the case of incompressible fluid, we have

ρV:V=Δp+2μΔV+:2μS¯;E22

if also μ=const,then

ρV:V=Δp.E23

Now we consider the general case of fluid motion, taking into account its compressibility.

The set of equations of motion of an incompressible fluid contains two—Navier–Stokes and continuity (one vector equation and one scalar equation) [2, 3]:

ρdVdt=p+μΔV+ρfV=0.E24

This set of two equations is closed: it contains two unknown quantities—velocity vector Vand pressure per two equations. The set describes laminar flows; in turbulent flows it becomes unclosed because Reynolds stress tensor appeared.

In case of compressible flows at ρconst, divergence of velocity is V0, and the Navier–Stokes equation (Eq. (19)) of a fluid motion at μ=consthas the form:

ρdVdt=p+μΔV+μV+ρf,E25

where pis defined by Eq. (17). Continuity equation is written in the form of Eq. (1). If ρconst, the set of equations (Eq. (25) and Eq. (1)) becomes unclosed, because density will also be unknown. To close the set of equation, energy equation is used, which contains one more unknown scalar quantity—temperature T. To determine temperature T, state equation is used; usually in fluid dynamics, it is the Mendeleev-Clapeyron equation. Energy equation could be written as the equation of specific internal energy transport:

ρdudt=q+σ¯:V+ρqs,E26

where u is the specific internal energy (for ideal gas it could be expressed with the help of the isochore heat capacity, du=cvdT); qis the heat flux vector (in laminar flow by Fourier’s law, q=λT); λ is the thermal conductivity of the material; and qsis the heat flux from internal or external sources.

Mendeleev-Clapeyron equation has the form

p=ρRT,E27

where R is the universal gas constant. In case of real gas or fluid, the state equation becomes more complicated.

For liquids it usually supposes ρ = const. This condition is applicable for gas motions and also in case the velocities of gas particles are less than 1/3 of sound velocity.

Eqs. (1), (25), (26), and (27) are valid for laminar regime of motion. In case of turbulent regime in these equations, correlations will appear, caused by velocity, density, and temperature pulsations. For closure of the set of equations of turbulent motion, additional relations are required.

4. Vorticity vector and its associated tensor

Vorticity ωis a vector quantity, which characterizes velocity field:

ω=12rotV=12×V,E28

in component form

ω=12Vjxiεkijek,

where εijk is the Levi-Civita tensor in component form. Components of ωvector are

ω1=ωx=12VzyVyz=12V3x2V2x3ω2=ωy=12VxzVzx=12V1x3V3x1ω3=ωz=12VyxVxy=12V2x1V1x2.E29

Vorticity vector ωand spin tensor Ω¯are connected with each other through Levi-Civita tensor 3ε¯=εijkeiejek. These quantities are mutually associated. They say that tensor Ω¯=12VVTis associated to vector ω=12×V, because the following relations are satisfied:

Ω¯:3ε¯=3ε¯:Ω¯=2ω=×V.E30

And vice versa, vector ωis associated with tensor Ω¯since the following expression is valid:

3ε¯ω=ω3ε¯=Ω¯.E31

In Eq. (30) spin tensor Ω¯is translated to the vector ω; in Eq. (31) vector ωis associated with spin tensor.

Let us prove expression Eq. (30):

Ω¯:3ε¯=12VVT:3ε¯=12VjxiVixjeiej:εpqkepeqek==12VjxiVixjεjikek=12εji1VjxiVixje1+12εji2VjxiVixje2++12εji3VjxiVixje3=12V2x3V3x2V3x2+V2x3e1++12V3x1V1x3V1x3+V3x1e2+12V1x2V2x1V2x1+V1x2e3==2ω1e12ω2e22ω3e3=2ω=×V.

The same for Eq. (31):

3ε¯ω=εijkeiejekωses=ωkεijkeiej=12Vsxtεktsεijkeiej.

Let us descry components of this second-rank tensor: when i=jthey are equal to zero; when i=1,j=2they are

12Vsxtεktsε12k=12Vsxtε3ts=12V2x1V1x2;

values for all i,j=1,2,3could be obtained by the same way.

The matrix of components of this tensor is

012V2x1V1x212V3x1V1x312V1x2V2x1012V2x1V1x212V1x3V3x112V2x3V3x20.

It can be seen that it is a matrix of components of the antisymmetric tensor Ω¯, which means that relation (31) is valid.

It is easy to see also that

ωΩ¯=0,ω×Ω¯=0,ω=0.E32

5. Vorticity transport equation

Rotation of convective acceleration of a fluid particle could be written as

×VV=2ωV2Vω.E33

Evidence of this equation can be performed by writing convective acceleration according to the formula:

VV=V22V××V.E34

Gradient of vorticity is the pseudo tensor of rank 2:

ω=12×V=esxs12Vjxiεkijek=122Vjxsxiεkijesek.E35

Trace of this tensor is trω=0. It is also possible to distinguish the symmetric and antisymmetric parts of this tensor:

142Vjxsxiεkij+2Vjxkxiεsijesek,142Vjxsxiεkij2Vjxkxiεsijesek.

Let us assume that the fluid is incompressible, μ = const, and its motion occurs in the field of potential mass forces. In this case with the help of Eq. (34), we can obtain the Navier–Stokes equation in the form:

Vt+V22+P+U+×V×V=νΔV;

now we apply curl operation (rot=×) to the left and right parts of this equation:

t×V+××V×V=νΔ×V.

We could rewrite the second term of the left part in this form:

V×V×VV+×VVV2ω,

but ω=0, and fluid is incompressible (V=0); therefore, this term finally can be written as

2Vω2ωV.

As a result, we can obtain transport equation of vortices in an incompressible viscous fluid, which is named as the generalized Helmholtz equation:

ωt+VωωV=νΔω,E36

or in more compact form:

dωdtωV=νΔω.E37

It is necessary to note that in the case of compressible fluid and at μconst, this equation becomes much more complicated.

This transport equation can be written in another form, considering the equality VωωV=×ω×V. Then

ωt+×ω×V=νΔω.E38

If we apply divergence operation to Eq. (36), then for incompressible fluid we obtain

ωt+VωωV=νΔω;

because ω=0, we have

VωωV=0.

On the other hand,

Vω=V:ω+Vω;ωV=V:ω+ωV,

and, finally, we have 0=0, i.e., we shall not obtain a new expression.

For the second power of vorticity, we can write

ω2=VT:VV:V,E39

and now, if we scalar multiply transport equation of vortices by ω:

ωωt+VωωV=ωνΔω;

then we obtain scalar transport equation of ω2:

dω2dtωω:V=νΔω2νωT:ω.E40

For incompressible fluid S¯=Ω¯because S¯=12ΔV+12Vand Ω¯=12ΔV12V.

As we already know V××V=2VΩ¯; therefore, Eq. (34) can be written as

VV=V22+2VΩ¯.E41

Let us write one more equation:

V××V=V2Ω¯=VVTVV==ViVixjViVjxiej=xjViVixjViVjxi=VixjVixj+Vi2VixjxjVixjVjxiVi2Vjxixj=VT:VV:V+VΔVVV.

Therefore,

V××V=VT:VV:V+VΔVVE42

This equation also can be written in the next form:

V××V=2Ω¯:V+2VΩ¯or

V××V=2Ω¯:Ω¯+2Ω¯:S¯+2VΩ¯.

One more interesting relation is

VV=VΩ¯+VS¯,

but as we already mentioned, V××V=2VΩ¯; therefore,

VS¯=V2212V××V.E43

The vector product of gradients of scalar functions gives us a vector; in terms of rotation of a vector function, we can write

f×φ=×fφ.E44

Really, the left part of this equation is a vector:

f×φ=fx2φx3fx3φx2e1+fx3φx1fx1φx3e2+fx1φx2fx2φx1e3,

and the right part is.

×fφ=eixi×fφxjej=ei×ejxifφxj=εkijxifφxjek==ε1ijxifφxje1+ε2ijxifφxje2+ε3ijxifφxje3==x2fφx3x3fφx2e1+x3fφx1x1fφx3e2+x1fφx2x2fφx1e3==fx2φx3fx3φx2e1+fx3φx1fx1φx3e2+fx1φx2fx2φx1e3.

Therefore, Eq. (44) is valid.

The vector product of gradients of scalar functions also can be written as

f×φ=12φffφ:3ε¯=fφ3ε¯.E45

Here we have in component form:

fφ3ε¯=fφxsesεkijekeiej=fφxkεkijeiej==etxtfφxkεkijeiej=xifφxkεkijej==xifφxkεki1e1+xifφxkεki2e2+xifφxkεki3e3==fx3φx2fx2φx3e1+fx1φx3fx3φx1e2+fx2φx1fx1φx2e3.

It is easy to see that this is equal to expression for f×φwith the minus sign.

6. Mechanical energy equation

Mechanical energy balance equation can be obtained as a scalar product of each member of Eq. (12) on velocity vector V:

VρVt+VV=Vσ¯+Vρf.E46

Transformations of the left part lead us to the following results:

VVt=VkektViei=VkVitekei=VkVitδki=VkVkt=12tVkVk=12V2t;
VVV=VkekVjxjViei=VkVjVixjekei==VkVjVixjδki=VkVjVkxj=Vjxj12VkVk=VV22.

It is easy to see that in sum the left part is the material derivative of kinetic energy of a fluid particle—quantity ddtV22. Then Eq. (46) takes the form:

ρddtV22=Vσ¯+Vρf.E47

Usually stress tensor is defined as the sum σ¯=pE¯+τ¯, where τ¯is the shear stress tensor. Then the first term of the right part of Eq. (46) takes the form:

Vσ¯=VpE¯+Vτ¯.

Now we can represent equation of mechanical energy balance (Eq. (46)) considering pE¯=pas follows:

ρddtV22=Vp+Vτ¯+ρVf.E48

The first member of the right part of Eq. (46) is power of stresses Vσ¯,which can be written in the form:

Vσ¯=Vσ¯σ¯:V.E49

It is easy to be proven if we rewrite this expression in component form in Cartesian coordinates. In this case the left part of Eq. (49) is

Vσ¯=Vkekeixiσsjesej=Vkekσsjxieiesej==Vkekσijxiej=Vkσijxiekej=Vkσikxi.

The first term of the right part of Eq. (49) in component form is

Vσ¯=Vsesσijeiej=Vsσijeseiej=Viσijej==ekxkViσijej=δkjxkViσij=xkViσik=Vixkσik+Viσikxk.

The second term of the right part of Eq. (49) in component form is

σ:V=σijeiej:Vsxkekes=σijVsxkejekeies==σijVsxkδjkδis=σijVixj=Vixkσik.

Finally Eq. (49) in component form is

Vkσikxi=Vixkσik+ViσikxkVixkσik.

Due to the symmetry of the stress tensor σ¯=σ¯T, this expression is an identity (i.e., the left side is equal to the right one). Indeed, the second term of the right-hand side of this relation, after re-designating the index i by k and vice versa, takes the form Vkσkixi, but σki=σik; therefore both parts of the expression are equal to each other. Thus, equality (49) is valid.

We could simplify the last term of the right part of Eq. (46) if we introduce potential Uof mass forces in field of gravity (z axis is positive upwards) as earlier f=U, U=gz=rg,where gis the gravity acceleration vector in the field of gravity. Then

Vρf=ρVU=ρdrdtU=ρ1dtUdr=ρdUdt.E50

After substituting the above expressions into Eq. (46), we obtain the equation for mechanical energy of a fluid flow:

ρddtV22+U=Vσ¯σ¯:V.E51

In the left part of this equation, we observe the total mechanical energy of a fluid flow as the sum of kinetic and potential energy of the flow [6]. Often the right part of Eq. (51) is written in another form, where stress tensor is written as the sum σ=pE¯+τ¯. Then the right part of Eq. (51) will have the form:

VpE¯+Vτ¯+pE¯:Vτ¯:V.E52

The first member is

VpE¯=Vieipδjkejek=Vipδjkδijek==pVkek=esxspVkek=pVkxsδsk=xkpVk==VkpxkpVkxk=VppV.

The third member is

pE¯:V=pδijeiej:Vsxkekes=pVsxkδijδjkδis=pVkxk=pV.

When we substitute these terms in Eq. (52) and then in Eq. (51), the equation for mechanical energy of a fluid flow will take the form:

ρddtV22+U=Vp+Vτ¯τ:V.E53

As a result, we could conclude that the rate of change of total mechanical energy of a flow is equal to the sum of the powers of the pressure forces and viscous friction.

Navier–Stokes equation for a steady flow of viscous incompressible fluid is

ρVV=p+μΔV+ρf.E54

The Laplacian of velocity in the right part can be written in the form:

ΔV=V××V.E55

It can be obtained by consideration of operation ××V:

××V=eixi×Vjxkεskjes==2Vjxixkεskjεlisel=2Vjxixkεskjε1ise1+2Vjxixkεskjε2ise2+2Vjxixkεskjε3ise3.

The member with the basis vector e1is determined as

2Vjxixkεskjε1is=2Vjx2xkε3kj2Vjx3ε2kj=2V2x2x12V1x3x3+2V3x3x1==x12V1x1+2V2x2+2V3x32V1x122V1x222V1x32=x1VΔV1.

The same can be written for the members with basis vectors e2and e3. As a result, we obtain

××V=x1VΔV1e1+x2VΔV2e2++x3VΔV3e3=VΔV.

And therefore formula Eq. (55) is valid.

One more useful expression based on Eq. (55) is

S¯=ΔV+V=2V××V.

Using Eqs. (34) and (55) and considering the mass force in field of gravity with the help of potential U, U=gz(z axis is positive upwards), we obtain instead Eq. (54):

V22V××V=1ρp+νVν××V+U,

where ν=μρis the kinematic (momentum) viscosity of fluid.

In incompressible fluid ρ=const, V=0and then we have

V22+pρ+gz=V××Vν××VVν××V.E56

The gradient of total mechanical energy of a fluid particle E=V22+pρ+gzdepends on vortex structure of the flow. When ×V=0the right part of Eq. (56) is zero, and then E=constin the whole area of the flow.

It is possible to obtain the divergence form of Eq. (54) for incompressible fluid considering V=0and using Eq. (55) and the relation:

VV=VV+VV.E57

Then Eq. (54) will take the form:

ρVV=p+ρUμ××V.E58

Using concepts of identity tensor I¯and Levi-Civita tensor 3ε¯=εijkeiejek, we can write members of the right part in the divergence form, and as a result, the whole Navier–Stokes equation for steady flow of incompressible fluid can be written as

ρVV+pI¯ρUI¯+ρν3ε×V=0.E59

The last term of Eq. (59) can be considered in a more simple form due to relation for incompressible fluid ΔV=V=S¯. Finally, the divergence form of the Navier–Stokes equation for steady flow of an incompressible fluid is

ρVV+p+ρgzI¯μS¯=0.E60

7. Energy equation for moving fluid

The first law of thermodynamics connects internal energy, heat, and work. In the case of moving fluid, it can be written as follows:

ρdudt=q+σ¯:V+qv,E61

where t is the time; u is the specific internal energy; qis the heat flux density vector due to thermal conductivity; σ¯is the stress tensor; and qvis the value of heat entering into the particle volume from action of external or internal sources per unit time. In this expression, the colon denotes double scalar product of tensors; in this case these are the stress tensor and velocity gradient tensor.

The physical meaning of this equation is that the rate of change of internal energy per unit volume is equal to rate of energy supply due to heat conduction, due to dissipation of mechanical energy of the flow, and due to heat from external or internal sources. Since stress tensor σ¯can be written as σ¯=pE¯+τ¯,where τ¯is the shear stress tensor, taking into account material derivative definition, we can rewrite Eq. (61) in this form:

ρut+Vu=qpV+τ¯:V+qv.E62

This is the energy equation in terms of transfer of specific internal energy u.

Vector qin the energy equation is determined by Fourier’s law:

q=λT,E63

where T is the temperature and λ is the coefficient of thermal conductivity.

Fourier’s law of thermal conductivity can also be written in terms of enthalpy, which for an ideal gas is related to temperature by the formula h=cpT, where ср is the isobar heat capacity. Then considering λ=ρcpa, where a is the thermal diffusivity, heat flux density vector can be written in the form:

q=λT=ρcpaT=ρνaνcpT=ρνPrh=μPrh,

where Pr=a/νis the Prandtl number.

In Cartesian coordinates Eq. (62) can be written as follows:

ρut+Vjuxj=xjλTxjpVjxj+τijVixj+qv.E64

The terms pVand τ¯:Vshow us in a moving fluid heating or cooling can occur. The term pVmay cause significant change of temperature, when gas expands (compresses) rapidly. The term τ¯:Vis always positive; it characterizes dissipation of mechanical energy and its transformation to heat energy. This scalar quantity is usually named as Rayleigh dissipation function [6] and denoted as τ¯:V=Ф. Let us write this function in Cartesian coordinates for Newtonian viscous fluid, when rheological relation has the form:

τ¯=23μVE¯+2μS¯,E65

where μ is the fluid shear viscosity and S¯is the strain rate tensor.

Now we could write the dissipative term τ¯:Vin Eq. (62) by simple transformations:

Ф=τ¯:V=23μVE¯+2μS¯:V==23μVE¯:V+2μ12V+VT:V==23μVδijeiej:Vsxkekes+μV:V+VT:V==23μVδijδjkδisVsxk+μVjxieiej:Vsxkekes+Vixjeiej:Vsxkekes==23μVVixi+μVjxiVsxkδjkδis+VixjVsxkδjkδis=23μV2++μVjxiVixj+VixjVixj=23μVixi2+μVjxiVixj+VixjVixj.

Thus, in component form Rayleigh function Фcan be written as

Ф=τ¯:V=23μVixi2+μVjxiVixj+Vixj:Vixj,E66

or in usual notations

Ф=μ23Vxx+Vyy+Vzz2+2Vxx2+Vyy2+Vzz2+Vxy+Vyx2+Vxz+Vzx2+Vyz+Vzy2.E67

This function can also be written in the componentless form:

Ф=τ¯:V=23μV2+μV:V+V:VT.E68

For perfect gases [6, 7] internal energy is connected with temperature by the relation du=cvdT, where cvis the isochore thermal capacity. Then, instead of Eq. (62) with the help of expression for vector q, we can write equation for temperature transport in the form:

ρcvTt+VT=λTpV+τ¯:V+qv.E69

The energy equation (Eq. (62)) can be also written in terms of enthalpy h=u+pρ. With this purpose we need to add the term ρddtpρto the left and right parts of the equation. Then we obtain in the left part ρdhdt, but in the right part, we shall get this term in transformed form shown as follows:

ρddtpρ=dpdtpρdρdt=dpdt+ρV.E70

Here we also used continuity equation (Eq. (2)). Finally, we can obtain energy equation in the form of enthalpy transport as

ρdhdt=q+dpdt+τ¯:V+qv.E71

This is the second form of energy equation for the perfect gas in which dh=cpdT, where cpis the isobar heat capacity, which leads to the following transport equation for temperature:

ρcpdTdt=λT+dpdt+τ¯:V+qv.E72

One more form of the energy equation can be written if we introduce stagnation enthalpy h+V22. To do it we need to add equations for mechanical energy (Eq. (48) to Eq. (71)); as a result we obtain the equation:

ρddth+V22=q+pt+τ¯V+ρVf+qv.E73

Here we used the relation:

τ¯V=Vτ¯+τ¯:V,E74

which is easy to be proven if we write it down in the component form considering symmetry of stress tensorτ.

As a result, the dissipative term in Eq. (73) can be written as follows:

τ¯V=Ψ+Ф,E75

where Фis the Rayleigh dissipation function and Ψ=Vτ¯is the scalar quantity, which can be named as additional dissipation function. This additional dissipation function in Cartesian coordinates for Newtonian Stokes liquid can be written as

Ψ=Vτ¯=V23μVE¯+2μS¯==Vekxk23μVδijeiej+2μSijeiej==Vxk23μVδijδkiej+2μSijδkiej==Vxk23μVek+2μSkjej==Vsesxk23μVek+2μSkjej==V23μV+Vjxk2μSkj.

In usual axis designations, the first term is

Vxx+Vyy+Vzz23μVxx+Vyy+Vzz,

while second term is

Vjxk2μSkj=V1xk2μSk1+V2xk2μSk2+V3xk2μSk3==V1x12μS11+x22μS21+x32μS31++V2x12μS12+x22μS22+x32μS32++V3x12μS13+x22μS23+x32μS33.

Finally function Ψin Cartesian coordinates can be written as follows:

Ψ=23VxxμV+VyyμV+VzzμV+Vxx2μVxx+yμVxy+Vyx+zμVzx+Vxz+VyxμVxy+Vyx+y2μVyy+zμVzy+Vyz+VzxμVzx+Vxz+yμVzy+Vyz+z2μVzz.E76

The fourth form of the energy equation can be written in terms of entropy s transport. According to the fundamental thermodynamic relation,

Tds=dh1ρdp.E77

Hence we have

Tdsdt=dhdt1ρdpdt,

and then if we substitute quantity dhdtfrom Eq. (77) to Eq. (71), we obtain

ρTdsdt=q+τ¯:V+qv.E78

All forms of the equation energy (in terms of internal energy, enthalpy, stagnation enthalpy, and entropy) are equivalent.

Equation for temperature field of an arbitrary gas in the form of equation of transport of temperature T can be obtained from Eq. (62) or Eq. (71). In these cases quantities dudtand dhdtfor arbitrary gases and liquids must be specified using known formulas, which follow from Maxwell’s relations:

du=cvdT1ρ2TpTρpdρ,E79
dh=cpdT+1ρ2ρ+TρTpdp.E80

The subscripts in derivatives here fix the parameters, with the constancy of which the derivatives are calculated. From these formulas the expressions for derivatives can be obtained:

dudt=cvdTdt1ρ2TpTρpdρdt,E81
dhdt=cpdTdt+1ρ2ρ+TρTpdpdt.E82

If we substitute them into Eq. (62) and Eq. (71), we obtain two forms of the equation energy in terms of temperature transport.

In heat transfer problems, boundary conditions are specified in three different kinds—the first, second, and third kind:

  1. The boundary conditions of the first kind consist in setting the temperature on the surface of the body.

  2. The boundary conditions of the second kind are setting of the distribution of the heat flux density q on the surface of the body.

  3. The boundary conditions of the third kind consist in setting the temperature of the flow over the surface of the body and the heat transfer conditions on its surface.

8. Divergence form of transport equations

Material derivative of any physical quantity Θ multiplied by density ρ always can be written in the “divergent” form as

ρdΘdt=tρΘ+ρVΘ.E83

This directly follows from the continuity equation [Eq. (2)].

Let us consider in detail the following cases for three ranks of a certain physical quantity Θ.

8.1 Quantity Θ is a scalar

Let us assume that quantity Θ is temperature T:

ρdTdt=tρT+ρVT.E84

We could prove this equality if we write the left and right parts in component form. For the left part, we have

ρdTdt=Tt+ρVT=ρTt+ρVjTxj.

For the right part, we have

tρT+ρVT=Tρt+ρTt+xjρVjT==Tρt+ρTt+TVjρxj+ρTVjxj+ρVjTxj==Tρt+Vjρxj+ρVjxjρt+Vρ+ρV=0+ρTt+ρVjTxj=ρTt+ρVjTxj.

Since the expression in parentheses is zero (due to continuity equation), the equality of the left and right parts is obvious.

8.2 Quantity Θ is a vector

Let us assume that quantity Θ is velocity V. In this case its material derivative can be written in the form:

ρdVdt=tρV+ρVV.E85

Here in the last term, we see tensor ρVV(momentum flow tensor); the sign of tensor multiplicationis omitted for ease of recording.

We could prove this equality if we write the left and right parts in the component form and use continuity equation.

For the left part, we have

ρdVdt=ρVt+ρVV=ρdVidtei+ρVjVixjei.

The first term of the right part is

tρV=tρViei=ρtViei+ρVitei.

The second term of the right part is

ρVV=ekxkρVjViejei=xkρVjVekejei==δkjxkρVjViei=xjρVjViei=ρVjxjViei+VjρxjViei+ρVjVixjei.

The right part as a whole is

ρVitei+ρVjVixjei+Vieiρt+Vjρxj+ρVjxjρt+Vρ+ρV=0.

Therefore, the expression (Eq. (83)) is valid in case Θ is a vector.

8.3 Quantity Θ is a tensor

Let us assume that Θ is a tensor, for instance, stress tensor σ¯. Stress tensor is a second-rank symmetric tensor, which in Cartesian coordinates can be written in the form σ¯=σijeiej. Let us prove the equality:

ρdσ¯dt=tρσ¯+ρVσ¯.E86

The left part of this equation in the component form can be written as follows:

ρdσ¯dt=ρddtσijeiej=ρtσijeiej+ρVσijeiej==ρσijteiej+ρVkσijxkeiej.

The right part is

tρσ¯+ρVσ¯=tρσijeiej+ekxkρVsσijeseiej==σijρteiej+ρσijteiej+δksxkρVsσijeiej==σijρteiej+ρσijteiej+xkρVkσijeiej==σijρteiej+ρσijteiej+Vkσijρxkeiej+ρσijVkxkeiej+ρVkσijxkeiej==ρσijteiej+ρVkσijxkeiej+σijeiejρt+Vkρxk+ρVkxk=0

Therefore, the expression (Eq. (83)) is also valid in case Θ is a tensor.

It is necessary to note the derivative ddtσ¯, which contains local and convective parts ddt=t+V, can, at first glance, be used in fluid models when writing the defining equation in the form of a differential transport Equation [2, 5]. However, careful analysis shows that the material derivative for a second-rank tensor is not an invariant quantity [5, 8, 9]. By this reason, instead of derivative ddt, derivative DDtis usually used as the material derivative for a second-rank tensor, which contains also rotational part (deviatoric stress rate), which provides symmetry relative to rotations. The rotational part cannot be written in divergent form.

There are different forms of deviatoric stress rate for an arbitrary second-rank tensorA, for instance:

Jaumann G.: A¯Ω¯+A¯Ω¯T, Ω¯—antisymmetric spin tensor.

Rivlin R.: A¯V+VTA¯.

Truesdell C.: VA¯+A¯VT+trVA¯.

Oldroyd J., Sedov L.I., etc. [8, 10, 11]

At present, the question of which derivative is more appropriate to use when constructing rheological equations is unclear. The most common is the rotational derivative by Gustav Jaumann. The corresponding material derivative in the form by Jaumann, for an arbitrary tensor of the second rank, has the form

DA¯Dt=A¯t+VA¯+A¯Ω¯+A¯Ω¯T.E87

Material derivative in the form by Rivlin is written as follows:

DA¯Dt=A¯t+VA¯+A¯V+A¯VT.E88

It is easy to see that Rivlin’s derivative differs from Jaumann’s one by the additional term A¯S¯+A¯S¯T, which is neutral by itself.

Rotational derivative of a symmetric tensor is also a symmetric tensor. As an example, let us consider the rotational derivative of strain-rate tensor and spin tensor:

S¯Ω¯+S¯Ω¯T=14V+VTVVT+VT+VVTV==12VTVVVT.

As a result, we have obtained the symmetrical second-rank tensor.

9. Conclusions

In this chapter, some applications of tensor calculus in fluid dynamics and heat transfer are presented. Typical transformations of equations and governing relations are discussed. Main conservation equations are given and analyzed. The governing equations of fluid motion and energy were obtained.

© 2020 The Author(s). Licensee IntechOpen. This chapter is distributed under the terms of the Creative Commons Attribution 3.0 License, which permits unrestricted use, distribution, and reproduction in any medium, provided the original work is properly cited.

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Dmitry Nikushchenko and Valery Pavlovsky (March 11th 2020). Fluid Motion Equations in Tensor Form, Advances on Tensor Analysis and their Applications, Francisco Bulnes, IntechOpen, DOI: 10.5772/intechopen.91284. Available from:

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