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Z. Suo
Finite Deformation: General Theory
The notes on finite deformation have been divided into two parts: special
cases (http://imechanica.org/node/5065) and general theory. In class I start
with special cases, and then sketch the general theory. But the two parts can be
read in any order.
Model a body by a field of material particles. We model a body by
a field of material particles. Each material particle can be named any way we
want. For example, we can use an English letter, a Chinese character, or a color.
To talk about how close two particles are, we choose to name each material
particle by its coordinate X when the body is in a particular state. We will call
this particular state of the body the reference state. Often we choose the
undeformed state the reference state. However, even without external loading, a
body may be under a field of residual stress. Thus, we may not be able to always
set the reference state as the undeformed state. Rather, any state of the body may
be used as a reference state. From now on, we will use the phase “the material
particle X” as shorthand for “the material particle whose coordinate is X when
the body is in the reference state”.
Field of deformation. At time t, the body deforms to a current state.
In the current state, the material particle X moves to a place with coordinate x.
The deformation of the body varies from time to time, and from material particle
to material particle. The time-dependent field
x = x (X , t )
characterizes the history of deformation of the body. A central aim of continuum
mechanics is to evolve the field of deformation x (X, t ) by using an equation of
motion.
The displacement, velocity, and acceleration of the material particle X at
time t are, respectively,
x (X , t ) − X ,
∂x (X , t )
,
∂t
∂ 2 x (X , t )
.
∂t 2
They are all time-dependent fields.
When a body deforms, does each material particle preserve its
identity? We have tacitly assumed that, when a body deforms, each material
particle preserves its identity. Whether this assumption is valid can be
determined by experiments. For example, we can paint a grid on the body. After
deformation, if the grid is distorted but remains intact, then we say that the
deformation preserves the identity of each particle. If, however, after the
deformation the grid disintegrates, we should not assume that the deformation
preserves the identity of each particle.
Whether a deformation of body preserves the identity of the particle is
subjective, depending on the size scale we paint the grid, and the time scale over
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which we look at the body. A rubber, for example, consists of cross-linked long
molecules. If our grid is over a size much larger than the individual molecular
chains, then deformation will not disintegrate the grid. By contrast, a liquid
consists of molecules that can change neighbors. A grid painted on a body of
liquid, no matter how coarse the grid is, will disintegrate over a long enough time.
Similar remarks may be made for metals undergoing plastic deformation. Also,
in many situations, the body will grow over time. Examples include growth of
cells in a tissue, and growth of thin films when atoms diffuse into the films. The
combined growth and deformation clearly does not preserve the identity of each
material particle.
In these notes, we will assume that the identity of each material particle is
preserved as the body deforms.
X+dX
x(X,t)
x(X+dX,t)
X
reference state
current state
Deformation gradient. Recall the definition of the stretch of a bar:
length in current state
.
stretch =
length in reference state
We now extend this definition to a body in three dimensions and undergoing
inhomogeneous deformation.
Consider two nearby material particles in the body. When the body is in
the reference state, the two particles occupy places with coordinates X and
X + dX . When the body is in the current state at time t, the two particles occupy
places with coordinates x (X, t ) and x (X + dX , t ) . The stretch is generalized to
the ratio
x i (X + dX , t ) − x i (X , t )
.
dX K
This object represents 9 ratios, and is given a symbol:
∂x (X , t )
FiK = i
.
∂X K
This tensor, known as the deformation gradient, is a time-dependent field,
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F (X , t ) . This equation is linear in the field of deformation, x (X, t ) .
As a body deforms, each material element of line both rotates
and stretches. We have motivated the definition of the deformation gradient by
using the analogy with the stretch of a bar. An slight variation of the theme will
shed a different light. Now focus on the vector connecting the two nearby
material particles, X and X + dX . When the body is in the reference state, the
vector between the two material particle is dX , which we call a material element
of line. When the body is in the current state, this element becomes
dx = x (X + dX , t ) − x (X , t ) .
Thus,
∂x (X , t )
dx i = i
dX K .
dX K
We have defined the partial derivative as the deformation gradient, so that
dx i = FiK (X , t )dX K ,
or
dx = F(X , t )dX .
Thus, the deformation gradient maps the vector between two nearby material
particles from the reference state to the current state.
When the body deforms, the element rotates, as well as stretches. In the
reference state, let dL be the length of the element, and M be the unit vector in
the direction of the element, namely,
dX = MdL .
In the current state, let dl be the length of the element, and m be the unit vector
in the direction of the element, namely,
dx = mdl
Recall that the stretch of an element is defined by
dl
λ=
.
dL
Combining the above four equations, we obtain that
λm = F (X , t )M .
In the current state at time t, once the field of deformation, x (X , t ) , is known, the
deformation gradient F(X , t ) can be calculated. For a material element in any
direction M, the above expression gives in the current state the direction of the
element, m(X ,t , M ) , and the stretch of element, λ (X ,t , M ) .
Green deformation tensor. We can also obtain an explicit expression
for λ (X ,t , M ) . Taking inner product of the vector λm = F(X , t )M , we obtain that
λ2 = MT CM .
where
C = FT F .
The time dependent field, C (X , t ) , known as the Green deformation tensor,
is symmetric and positive-definite. In the current state at time t, once the field of
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deformation, x (X , t ) , is known, the tensor C (X , t ) can be calculated, and so can
the stretch of any material element of line, λ (X ,t , M ) .
Conservation of mass. When a body is in the reference state, a
material occupies a place with coordinate X, and a material element of volume
around the particle is denoted by dV (X ) . When the body is in a current state at t ,
let ρ be the nominal mass density, namely,
mass in current state
.
ρ=
volume in reference state
During deformation, we assume that a material particle does not gain to lose
mass, so that the nominal density ρ is time-independent. If the body in the
reference state is inhomogeneous, the nominal density in general varies from one
material particle to another. We write the nominal density as a function
ρ = ρ (X ) .
Thus, ρ (X )dV (X ) is the mass of the material element of volume at all time. The
total mass of the body is
ρ (X )dV .
∫
The integral extends to the entire volume of the body in the reference state. In
our theory, the nominal mass density is given.
In our previous work, we have been talking about the three ingredients of
solid mechanics (i.e., deformation geometry, force balance, and material model).
We have tacitly assumed that mass is conserved during deformation. The above
paragraph makes this additional ingredient explicit.
Conservation of linear momentum. In the current state, the linear
momentum of a material element of volume is
∂x (X , t )
ρ (X )
dV (X ) .
∂t
By conservation of linear momentum we mean that, for any part of the body and
at all time, the total force on the part equals the rate of change of the linear
momentum of the part. We next express this principle in useful terms.
Body force. Consider a material element of volume around material
particle X. When the body in the reference state, the volume of the element is
dV (X ) . When the body is in the current state at time t, the force acting on the
element of volume is denoted as B(X , t )dV (X ) , namely,
force in current state
B(X , t ) =
.
volume in reference state
This force is called the body force, and the vector B(X , t ) the density of the body
force. The body force is applied by an agent external to the body, and is given in
our theory.
Traction. Consider a material element of area at material particle X.
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When the body is in the reference state, the area of the element is A(X ) , and the
unit vector normal to the element is N(X ) . When the body is in the current state
at time t, the force acting on the element of area is denoted as T (X , t )dA(X ) ,
namely,
force in current state
T (X , t ) =
.
area in reference state
This force is called the surface force or traction. For a material element of area
on the external surface, the traction may be prescribed by an agent external to the
body, and is known in our theory. For a material element inside the body, the
traction represents the force exerted by one material particle on its neighboring
material particle. In this case, the traction is internal to the body, and need be
determined by the theory.
s31
C=dX3
s11
B=dX2
s21
A=dX1
Stress. When a bar is pulled by a force, the nominal stress is defined as
the force in the current state divided by the area of the cross section of the bar in
the reference state. We now generalize this definition to three dimensions. A
block of material is a rectangle in the reference state, and deforms into some
other shape in the current state. Consider a specific material element of area.
The element is normal to the axis X K when the block is in the reference state, and
moves to a new place and a new orientation when the block is in the current state.
In the current state, a force acts on the material element of area. Define the
nominal stress siK as the component i of the force acting on the material element
of area in the current state divided by the area of the material element of area in
the reference state. That is, siK is defined as the traction vector in the current
state acting on a material plane which is normal to the axis X K when the body is
in the reference state.
Conservation of linear momentum stipulates that, for any part of a body
and at any time, the force acting on the part equals the rate of change in the linear
momentum, namely,
d
∂x (X , t )
ρ (X )
T (X , t )dA + B(X , t )dV =
dV .
dt
∂t
∫
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The integrals extend over the surface and the volume of any part of the body. We
next derive from the conservation of linear momentum two consequences.
Stress-traction relation. Consider a material element of tetrahedron.
When the body is in the reference state, the four faces of the tetrahedron are
triangles: the three triangles on the coordinate planes, and one triangle on the
plane normal to the unit vector N. Let the areas of the three triangles on the
coordinate planes be AK , and the area of the triangle normal to N be A. The
geometry dictates that
AK = N K A .
When the body is in the current state, the tetrahedron deforms to a shape
of four curved faces. This deformed tetrahedron in the current state is a freebody diagram. Now apply the conservation of momentum to this deformed
tetrahedron. Acting on each of the four faces is a surface force. As the volume of
the tetrahedron decreases, the ratio of area over volume becomes large, so that
the surface forces prevail over the body force and the change in the linear
momentum. Consequently, the surface forces on the four faces of the tetrahedron
must balance, giving
siK AK = Ti A .
A combination of the above two equations give
siK N K = Ti .
Consequently, the nominal stress is a linear operator that maps the unit vector
normal to a material plane in the reference state to the traction acting on the
material plane in the current state.
Conservation of linear momentum in differential form. Consider any
part of the body. The force due to traction is
∂siK (X , t )
Ti (X , t )dA = siK (X , t )N K (X )dA =
dV .
∂X K
The first equality comes from the stress-traction relation, and the second equality
invokes the divergence theorem.
Consequently, conservation of linear
momentum requires that
∂siK (X , t )
d
∂x (X , t )
dV + Bi (X , t )dV =
dV .
ρ (X ) i
∂X K
dt
∂t
This equation holds for arbitrary part of the body, so that the integrands must
equal:
∂siK (X , t )
∂ 2 x i (X , t )
.
+ Bi (X , t ) = ρ (X )
∂X K
∂t 2
This equation is linear in the field of stress and the field of deformation.
An alternative derivation of the above equation goes as follows. Consider
a block of material ABC. When the body is in the reference state, the block is
rectangular. When the body is in the current state, the block deforms to some
other shape. Conserving linear momentum of this free-body diagram, we obtain
that
∫
∫
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∫
∫
∫
∫
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BCsi 1 (X 1 + A, X 2 , X 3 , t ) − BCsi 1 (X 1 , X 2 , X 3 , t )
+ CAsi 2 (X 1 , X 2 + B, X 3 , t ) − CAsi 2 (X 1 , X 2 , X 3 , t )
+ ABsi 3 (X 1 , X 2 , X 3 + C , t ) − ABsi 3 (X 1 , X 2 , X 3 , t )
+ ABCBi (X , t )
∂ 2 x i (X , t )
∂t 2
Divide this equation be the volume ABC, and we obtain that
∂siK (X , t )
∂ 2 x i (X , t )
+ Bi (X , t ) = ρ (X )
.
∂X K
∂t 2
= ABCρ (X )
Conservation of angular momentum. This principle stipulates that,
for any part of a body and at any time, the moment acting on the part equals the
rate of change in the angular momentum, namely,
d
∂x (X , t )
x (X , t )× T (X , t )dA + x (X , t )× B(X , t )dV =
x (X , t )×
ρ (X )dV .
dt
∂t
The first term can be converted into a volume integral as follows:
∂ (x j s pK )
ε ijp x j Tp dA = ε ijp x j s pK N K dA = ε ijp
dV
∂X K
∫
∫
∫
∫
∫
∫
∂x j
∂s ⎤
⎡
= ⎢ε ijp s pK
+ ε ijp x j pK ⎥ dV
∂X K
∂X K ⎦
⎣
Combining the above two equations, and using the equation for conservation of
linear momentum, we obtain that
∂x j
ε ijp s pK
dV = 0 .
∂X K
This equation holds for arbitrary part of the body, so that the integrand must
vanish:
∂x j
ε ijp s pK
= 0.
∂X K
∫
∫
This equation is equivalent to
sF T = Fs T .
That is, conservation of angular momentum requires that the product sF T be a
symmetric tensor. In general, neither the deformation gradient F, nor the
nominal stress s, is a symmetric tensor.
An alternative derivation of the above equation goes as follows. Consider
a small block in a body. In the reference state, the block is rectangular, of lengths
A, B, C . In the current state, the block deforms to some other shape. Consider
the free-body diagram of the block in the current state: a pair of forces si 1 BC act
on the pair of the material elements of area BC , a pair of forces si2CA act on the
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pair of the material elements of area CA, and a pair of forces si3 AB act on the
pair of the material elements of area AB .
In the current state, in the coordinate plane (i , j ) , we balance the
moments of the forces acting on the block:
BCsi 1 x j (X 1 + A, X 2 , X 3 , t ) − x j (X 1 , X 2 , X 3 , t )
[
]
+ CAs [x (X , X + B, X , t ) − x (X , X , X , t )]
+ ABs [x (X , X , X + C , t ) − x (X , X , X , t )]
= BCs [x (X + A, X , X , t ) − x (X , X , X , t )]
+ CAs [x (X , X + B, X , t ) − x (X , X , X , t )]
+ ABs [x (X , X , X + C , t ) − x (X , X , X , t )]
i2
j
1
2
3
i3
j
1
2
j1
i
1
j2
i
1
2
j3
i
1
2
j
1
2
3
j
1
2
3
3
2
3
i
1
2
3
3
i
1
2
3
i
1
2
3
3
Divide the equation by the volume ABC, and we obtain that
siK F jK = s jK FiK .
Virtual displacement and virtual work. Consider a field of virtual
deformation,
δx = δx (X ) .
The field virtual deformation is an arbitrary field, and has nothing to do with the
field of axial deformation x (X , t ) . In particular, the virtual displacement has
nothing to do with time.
Associated with the virtual deformation, we define the virtual deformation
gradient by
∂δx i (X )
δFiK =
.
∂X
The virtual deformation gradient is also a field, δF(X ) .
Consider any part of the body. Associated with the field of virtual
deformation δx (X ) , the surface force, the body force, and the inertial force
together do the virtual work
Tiδx i dA + Biδx i dV − ρx&&iδx i dV ,
∫
∫
∫
Using the divergence theorem, we convert the virtual work by the surface force
into an integral
siK N K δx i dA = (siK δx i ),K dV = siK ,K δx i + siK δx i ,K dV .
∫
∫(
∫
)
Recall conservation of linear momentum, and we find that the virtual work done
by all the forces reduces to
siK δx i ,K dV .
∫
This equation holds for any arbitrary part of the body. Consequently,
virtual work in the curent state
= siK δFiK .
volume in the reference state
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Hyperelastic material. Imagine that the block in the current state
undergoes a virtual deformation δx i (X ) . Define the virtual deformation gradient
by
∂δx i (X )
δFiK =
.
∂X K
Let W be the free energy of the block in the current state divided by the volume of
the block in the reference state. As a material model, we assume that the freeenergy density is a function of the deformation gradient, W(F). Define the virtual
change in the free energy density by
∂W (F )
δW = W (F + δF ) − W (F ) =
δFiK .
∂FiK
For a hyperelastic material, the virtual work done by all the forces acting
on the block equals the virtual change in the free energy:
δW = siK δFiK .
A comparison of the two expressions of the virtual change in the free energy gives
that
∂W (F )
siK =
.
∂FiK
This equation relates the stress to the deformation gradient once the function
W(F) is prescribed.
The free-energy density is unchanged if the body undergoes a
rigid-body rotation. The free energy is invariant if the particle undergoes a
rigid body rotation. Thus, W depends on F only through the combination
C KL = FiK FiL ,
or
C = FT F .
We write
W (F ) = Ω(C ) .
Recall that the stress is work-conjugate to the deformation gradient.
Using the chain rule in differential calculus, we obtain that
∂W (F ) ∂Ω(C ) ∂C MN
=
siK =
,
∂FiK
∂C MN ∂FiK
or
∂Ω(C )
siK = 2 FiL
.
∂C LK
Note that this equation automatically conserves angular momentum:
siK F jK = s jK FiK .
Tensor of tangent modulus for a hyperelastic material. Recall
that the tensor of tangent modulus is defined by
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K iKjL =
Z. Suo
∂siK (F )
.
∂F jL
Thus, for a hyperelastic material, the tensor of tangent modulus relates to the
free-energy density as
∂W (F )
K iKjL =
.
∂FiK ∂F jL
Consequently, for a hyperelastic material, the tensor of tangent modulus
possesses the major symmetry:
K iKjL = K jLiK .
An alternative formulation of hyperelasicity. Consider a body
subject to a field of body force B(X , t ) , a field of traction T (X , t ) , and a field of
&& (X , t ) . The traction is prescribed on part of the surface of the
inertial force − ρx
body, while the remainder of the surface is prescribed with displacement.
In the current state, let δx (X ) be a field of virtual displacement. The
virtual displacement vanishes on the part of the surface where the displacement is
prescribed, and is otherwise arbitrary.
By a hyperelastic material we mean that the material is modeled by an
energy density W (F ) , and that the virtual change in the energy of the body equals
the virtual work done by all the forces:
∂W (F )
δx i ,K dV = (Bi − ρx&&i )δx i dV + Tiδx i dA .
∂FiK
This equation is the basis for the finite element method.
To ensure that the free energy is invariant when the body undergoes a
rigid-body rotation, we require that W depend on F only through the Green
deformation tensor C = F T F .
We next show that the above equation conserves linear and angular
momentum. Using the divergence theorem, we rewrite the virtual change in the
energy of the body as
⎡ ∂W (F ) ⎤
∂W (F )
∂ ⎡ ∂W (F ) ⎤
δx i ,K dV = −
⎢
⎥δx i dV + ⎢
⎥ N K δx i dA .
∂FiK
∂X K ⎣ ∂FiK ⎦
⎣ ∂FiK ⎦
∫
∫
∫
∫
∫
∫
Because the virtual change in the energy equals the virtual work for any arbitrary
field of virtual displacement, we conclude that
∂ ⎡ ∂W (F ) ⎤
⎢
⎥ + Bi = ρx&&i
∂X K ⎣ ∂FiK ⎦
for every material particle in the volume, and
⎡ ∂W (F ) ⎤
⎢
⎥ N K = Ti
⎣ ∂FiK ⎦
for every material particle on the surface of the body where the traction is
prescribed. These equations recover those for conservation of linear momentum
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once we identify
∂W (F )
.
∂FiK
Angular momentum is conserved once we require that W depends on F only
through the Green deformation tensor C = F T F .
siK =
Incompressible material. Rubbers and metals can undergo large
change in shape, but very small change in volume. A commonly used idealization
is to assume that such materials are incompressible, namely,
det F = 1 .
In arriving at siK = ∂W (F ) / ∂FiK , we have tacitly assumed that each component of
FiK can vary independently. The condition of incompressibility places a
constraint among the components. To enforce this constraint, we replace the
free-energy function W (F ) by a function
W (F ) − Π (det F − 1 ) ,
with Π as a Lagrange multiplier. We then allow each component of FiK to vary
independently, and obtain the stress from
∂
[W (F ) − Π(det F − 1)] .
siK =
∂FiK
Recall an identity in the calculus of matrix:
∂ det F
= H iK det F ,
∂FiK
where H is defined by H iK FiL = δ KL and H iK F jK = δ ij .
Thus, for an incompressible material, the stress relates to the deformation
gradient as
∂W (F )
− ΠH iK det F .
siK =
∂FiK
The Lagrange multiplier Π is not a material parameter. For a given boundaryvalue problem rather, Π is to be determined as part of the solution.
Neo-Hookean material. For a neo-Hookean material, the free-energy
function takes the form
W (F ) =
µ
FiK FiK .
2
The material is also taken to be incompressible, namely,
det F = 1 .
The stress relates to the deformation gradient as
siK = µFiK − H iK Π .
Perturb an equilibrium state of finite deformation. A body is
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made of a material characterized by a relation between the stress and the
deformation gradient:
siK = giK (F ) .
The body is subject to a dead load B(X ) in the volume. One part of the surface of
the body is subject to dead load T (X ) , and the other part of the surface is held at
prescribed place.
Let x 0 (X ) be a state of equilibrium compatible with the above
prescriptions. Associated with this state is the deformation gradient
∂x 0 (X )
,
FiK0 = i
∂X K
and the stress
0
siK
= giK (F 0 ) .
The stress field balances the forces
0
(X ) + B (X ) = 0
∂siK
i
∂X K
in the volume of the body, and
0
siK
(X )N K (X ) = Ti (X )
on the part of surface where the traction is prescribed. On the part of the surface
where the place is prescribed, x 0 (X ) is held at the prescribed place.
When the state of equilibrium, x 0 (X ) , is now perturbed by an
infinitesimal deformation, u(X , t ) , the field of deformation becomes
x (X , t ) = x 0 (X ) + u(X , t ) .
Associated with this field of deformation is the deformation gradient
∂u (X , t )
FiK (X , t ) = FiK0 (X ) + i
,
∂X K
and the stress
∂u (X , t )
siK (F ) = siK (F 0 ) + K iKjL (F 0 ) j
.
∂X L
Here we have expanded the stress into the Taylor series up to terms linear in the
perturbation. Recall the equation of force balance
∂2 x
∂siK
+ Bi = ρ 2 i .
∂t
∂X K
Inserting the stress-strain relation into the equation of force balance, we obtain a
homogeneous partial differential equation:
∂u j (X , t ) ⎤
∂ 2 ui (X , t )
∂ ⎡
0
.
⎥ = ρ (X )
⎢ K iKjL (F )
∂t 2
∂X K ⎣
∂X L ⎦
The boundary conditions also homogeneous:
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K iKjL (F 0 )
∂u j (X , t )
∂X L
Z. Suo
NK = 0
on the part of the surface where the dead force T (X ) is prescribed, and
u(X , t ) = 0
on the part of the surface where the place is prescribed. These equations are
solved subject to an initial condition.
The equation of motion for the perturbation u(X , t ) looks similar to that
in linear elasticity. Thus, solutions in linear elasticity may be reinterpreted for
phenomena of this type. We give examples below.
Linear vibration around a state of equilibrium. We have already
analyzed the vibration of beam subject to an axial force. In general, we look for
solution of the form
u(X , t ) = a (X )sin ωt ,
where ω is the frequency, and a(X ) is the field of amplitude. The equation of
motion becomes that
∂a j (X ) ⎤
∂ ⎡
0
2
⎥ = − ρ (X )ω ai (X ) .
⎢ K iKjL (F )
∂X K ⎣
∂X L ⎦
This equation, in conjunction with the homogeneous boundary conditions, forms
an eigenvalue problem. The solution to this eigenvalue problem determines ω
and a(X ) for a set of normal modes.
Plane waves superimposed on a homogeneous deformation in
an infinite body. When a bar is subject to uniaxial tension, homogenous
deformation satisfies all governing equations.
However, the state of
homogeneous solution may not be the only solution. Necking is an alternative
solution, a bifurcation from the homogenous deformation. In the previous
analysis, we have just considered the homogenous deformation, and have
identified the onset of necking with the axial force in the force-strain curve peaks.
Now we wish to push the analysis a step further: we wish to consider the possible
small perturbation from a homogenous deformation.
Consider an infinite body. Assume a plane wave of small amplitude:
u(X , t ) = af (N ⋅ X − ct ) ,
where a is the unit vector in the direction of displacement, N the unit vector in
the direction of propagation, c the wave speed, and f the wave form.
The equation of motion becomes
K iKjL (F 0 )N K N L a j = ρc 2 ai .
This is an eigenvalue problem.
When the modulus of tangent modulus possesses the major symmetry,
K iKjL = K jLiK , the acoustic tensor K ikjL N K N L is also symmetric. According to a
theorem in linear algebra, this symmetric acoustic tensor will have three real
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eigenvalues, and the three eigenvectors are orthogonal to one another.
Furthermore, when the acoustic tensor is positive-definite, the three eigenvalues
are positive, leading to three distinct plane waves.
Exercise. An infinite body of an incompressible material cannot support
longitudinal wave, but can support shear wave. Assume that the body is in a
homogeneous state of uniaxial stress. A small disturbance propagates along the
axis of stress as a shear wave. Determine the speed of this shear wave.
Bifurcation. The tensor of tangent modulus depends on the state of
homogeneous deformation, K iKjL (F 0 ) , and may no longer be positive-definite.
When the tangent modulus reaches the critical condition
det K iKjL (F 0 )N K N L = 0
[
]
in some direction N, we can find a nonvanishing displacement a at c = 0. This
equation may be regarded as a 3D generalization of the Considère condition.
Reading. J. R. Rice, "The Localization of Plastic Deformation", in
Theoretical and Applied Mechanics (Proceedings of the 14th International
Congress on Theoretical and Applied Mechanics, Delft, 1976, ed. W.T. Koiter), Vol.
1, North-Holland Publishing Co., 1976, 207-220.
http://esag.harvard.edu/rice/062_Rice_LocalPlasDef_IUTAM76.pdf
Surface instability of rubber in compression, M. A. Biot, Appl. Sci.
Res. A 12, 168 (1963). A semi-infinite block of a neo-Hookean material is in a
homogeneous state of deformation, with λ1 and λ2 being the stretches in the
directions parallel to the surface of the block, and λ3 being the stretch in the
direction normal to the surface. The material is taken to be incompressible, so
that λ1 λ2 λ3 = 1 . The compression in direction 1 is taken to be more severe than
that in direction 2, so that when the surface wrinkles in one orientation, leaving
λ2 unchanged. That is, the wrinkled block is in a state of generalized plane strain.
Biot found the critical condition for this instability:
λ3 / λ1 = 3.4
The analysis of this problem is analogous to that of the Rayleigh wave.
Polar decomposition. We next consider a number of refinements of
the theory. By definition, the deformation gradient is a linear operator that maps
one vector to another vector. For any linear operator there is a theorem in linear
algebra called polar decomposition. Any linear operator F can be written as a
product:
F = RU ,
where R is an orthogonal operator, satisfying R T R = I , and U is calculated from
FT F = U 2 .
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Thus, U is symmetric and positive-definite.
Lagrange strain. Define the Lagrange strain E KL by
dl 2 − dL2 = E KL dX K dX L .
Recall
dL2 = dX K dX K ,
and
dl 2 = FiK FiL dX K dX L
We obtain that
1
(FiK FiL − δ KL ) ,
2
where δ KL = 1 when K = L, and δ KL = 0 when K ≠ L . The E KL tensor is symmetric.
The three tensors are related as
1
E = (C − I ), C = U 2
2
E KL =
Exercise. The Lagrange strain forms a link between finite deformation
and the infinitesimal deformation approximation. Let the displacement field be
U (X , t ) = x (X , t ) − X ,
Show that the Lagrange strain is
1 ⎛ ∂U K ∂U L ∂U i ∂U i ⎞
⎟.
+
+
E KL = ⎜⎜
2 ⎝ ∂X L ∂X K ∂X K ∂X L ⎟⎠
Thus, the Lagrange strain coincides with the strain obtained in the infinitesimal
strain formulation if
∂U i
<< 1 .
∂X K
This in turn requires that all components of linear strain and rotation be small.
However, even when all strains and rotations are small, we still need to balance
force in the deformed state, as remarked before.
Exercise. We can relate the general definition of the Lagrange strain to
that introduced in the beginning of the notes for a tensile bar. Consider a
material element of line in a three dimensional body. In the reference state, the
element is in the direction specified by a unit vector M. In the current state, the
stretch of the element is λ . We have defined the Lagrange strain in one
dimension by
λ2 − 1
.
η=
2
Show that the Lagrange strain of the element in direction M is given by
η = E KL M K M L .
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Exercise. The tensor of Lagrange strain can also be used to calculate the
engineering shear strain. Consider two material elements of line. In the
reference state, the two elements are in two orthogonal directions M and N . In
the current state, the stretches of the two elements are λM and λN , and the angle
between the two elements become
shear strain. Show that
π
2
sin γ =
− γ . We have defined γ as the engineering
2 E KL M K N L
λM λN
.
Deformation of a material element of volume.
dV = dX 1 dX 2 dX 3 be an element of volume in the reference state.
Let
After
deformation, the line element dX 1 becomes dx 1 , with components given by
dx i1 = Fi 1 dX 1 .
We can write similar relations for dx 2 and dx 3 . In the current state, the volume
of the element is
dv = (dx 1 × dx 2 )⋅ dx 3 .
We can confirm that this expression is the same as
dv = det (F )dV .
Deformation of a material element of area. Let an element of area
be NdA in the reference state, where N is the unit vector normal to the element
and dA is the area of the element. After deformation, the element of area
becomes nda in the current state, where n is the unit vector normal to the
element and da is the area of the element. An element of length dX in the
reference state becomes dx in the current state. The relation between the
volume in the reference state and the volume in the current state gives
dx ⋅ nda = det (F )dX ⋅ NdA ,
or
dX K FiK ni da = det(F )dX K N K dA .
This relation holds for arbitrary dX , so that
FiK ni da = det(F )N K dA ,
or, in vector form,
F T da = det (F )dA .
The second Piola-Kirchhoff stress. Define the tensor of the second
Piola-Kirchhoff stress, S KL , by
virtual work in the curent state
= S KLδE KL .
volume in the reference state
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This expression defines a new measure of stress, S KL . Because E KL is a
symmetric tensor, S KL should also be symmetric. Recall that we have also
expressed the same virtual work by siK δFiK . Equating the two expressions for the
virtual work,
S KLδE KL = siK δFiK .
Recall definition of the Lagrange strain,
1
E KL = (FiK FiL − δ KL ) .
2
We obtain that
1
δE KL = (FiLδFiK + FiK δFiL )
2
and
siK = S KL FiL .
For a hypoelastic material, the free energy is a function of the Lagrange
strain, Ω(E ) . The second Piola-Kirchhoff stress is work-conjugate to the
Lagrange strain:
∂Ω(E )
S KL =
.
∂E KL
Lagrangian vs. Eulerian formulations. The above formulation uses
the material coordinate X as the independent variable. The function x (X , t ) gives
the place occupied by the material particle X at time t. This formulation is known
as Lagrangian. The inverse function, X (x , t ) , tells us which material particle is at
place x and time t. The formulation using the spatial coordinate x is known as
Eulerian. In the above, we have used the Eulerian formulation to study cavitation
because we know the current configuration. In general, the current configuration
is unknown, and we have used the Lagrangian formulation to state the general
problem. In the following, we list a few results related to the Eulerian
formulation.
Time derivative of a function of material particle. At time t, a
material particle X moves to position x (X, t ) . The velocity of the material
particle is
∂x (X , t )
.
V (X , t ) =
∂t
If we would like to use x as the independent variable, we change the variable
from X to x by using the function X (x , t ) , and then write
v (x , t ) = V (X , t ) .
Let G (X , t ) be a function of material particle and time. For example, G
can be the temperature of material particle X at time t. The rate of change in
temperature of the material particle is
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∂G (X , t )
.
∂t
This rate is known as the material time derivative. We can calculate the material
time derivative by an alternative approach. Change the variable from X to x by
using the function X (x , t ) , and write
g(x , t ) = G (X , t )
Using chain rule, we obtain that
∂G (X, t ) ∂g(x , t ) ∂g(x , t ) ∂x i (X , t )
+
=
.
∂x i
∂t
∂t
∂t
Thus, we can calculate the substantial time rate from
∂G (X , t ) ∂g(x , t ) ∂g(x , t )
vi (x , t ) .
=
+
∂t
∂t
∂x i
Let us applies the idea to the acceleration of a material particle. In the
Lagrangean formulation, the acceleration is
∂V (X , t ) ∂ 2 x (X , t )
.
=
A (X , t ) =
∂t
∂t 2
In the Eulerian formulation, the acceleration of a material particle is
∂v (x , t ) ∂vi (x , t )
ai (x , t ) = i
v j (x , t ) .
+
∂x j
∂t
Conservation of mass. In the Lagrange formulation, the nominal
mass density is defined by
mass in current state
ρR =
.
volume in reference state
That is, ρ R dV is the mass of a material element of volume. A subscript is added
here to remind us that the volume is in the reference state.
In the Eularian formulation, the true mass density is defined by
mass in current state
ρ=
.
volume in current state
That is, ρdv is the mass of a spatial element of volume.
The two definitions of density are related as
ρ R dV = ρdv ,
or
ρ R = ρ det F .
Conservation of mass requires that the mass of the material element of
volume be time-independent. Thus, the nominal density can only vary with
material particle, ρ R (X ) , and is time-independent. By contrast, the true density
is a function of both place and time, ρ (x , t ) . Conservation of mass requires that
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∂ρ (x , t ) ∂
[ρ (x, t )vi (x, t )] = 0 .
+
∂x i
∂t
When the material is incompressible, det F = 1 , we obtain that
ρ R (X ) = ρ (x , t ) .
True strain. Recall the definition of the true strain in one dimension.
When the length of a bar changes by a small amount from l (t ) to l + δl , the
increment in the true strain is defined as
δl
δε = .
l
Now consider a body undergoing a deformation x (X , t ) . Imagine a virtual
displacement δu(x ) in the current state. Consider two nearby material particles
in the body. When the body is in the reference state, the coordinates of the two
particles are X and X + dX . The vector dX is a material element of line. When
the body is in the current state at time t, the two material particles occupy places
x (X , t ) and x (X + dX , t ) , so that the vector between the two particles is
dx = x (X + dX , t ) − x (X , t ) .
Consider a material element of line. In the reference state, the element is
dX = MdL , where dL is the length of the element, and M is the unit vector in the
direction of the element. In the current state, the element becomes dx = mdl ,
where dl is the length of the element, and m is the unit vector in the direction of
the element.
The length of a material element of line at time t is
dl 2 = dx i dx i
Subject to the virtual displacement, the above equation becomes
dlδ (dl ) = d (δui )dx i .
Note that
∂ (δui )
d (δui ) =
dx j
∂x j
and
δε =
Thus,
δε =
δ (dl )
dl
.
∂ (δui )
mi m j
∂x j
This is the virtual increment of the strain of the material element of line. Only the
symmetric part
1 ⎡ ∂ (δui ) ∂ (δu j )⎤
+
⎢
⎥
∂x i ⎦⎥
2 ⎣⎢ ∂x j
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will affect the virtual increment of the strain of the material element of line. This
tensor generalizes the notion of the true strain, and is given the symbol:
1 ⎡ ∂ (δui ) ∂ (δu j )⎤
δε ij (x , t ) = ⎢
+
⎥.
2 ⎣⎢ ∂x j
∂x i ⎦⎥
Rate of deformation. Let v (x , t ) be the field of true velocity in the
current state. The same line of reasoning shows that the tensor
d ij (x , t ) =
1 ⎡ ∂vi (x , t ) ∂v j (x , t ) ⎤
+
⎢
⎥
∂x i ⎦⎥
2 ⎣⎢ ∂x j
allows us to calculate the rate of change the length of material element of line,
namely,
1
∂[dl (X , t )]
= dij mi m j .
dl (X , t )
∂t
The tensor dij is known as the rate of deformation.
Force balance. The true stress obeys that
⎡ ∂v (x , t ) ∂vi (x , t )
⎤
∂σ ij (x , t )
+
+ bi (x , t ) = ρ (x , t )⎢ i
v j (x , t )⎥ ,
∂x j
∂x j
⎢⎣ ∂t
⎥⎦
in the volume of the body, and
σ ij n j = t i
on the surface of the body. These are familiar equations used in fluid mechanics.
Relation between true stress and nominal stress.
definition of the nominal stress
virtual work in the curent state
= siK δFiK ,
volume in the reference state
and the definition of the true stress
virtual work in the curent state
= σ ijδε ij .
volume in the current state
Equating the virtual work on an element of material, we obtain that
σ ijδε ij dv = siK δFiK dV .
Recall the
Because the true stress is a symmetric tensor, we obtain that
∂δui (x )
σ ijδε ij = σ ij
.
∂x j
Also note that
∂δU i (X ) ∂δui (x ) ∂x j (X , t ) ∂δui (x )
F jK (X , t ) ,
δFiK =
=
=
∂x j
∂x j
∂X K
∂X K
and that
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dv / dV = det(F ) .
Insisting that the two expressions for the virtual work be the same for all virtual
motion, we obtain that
s F
σ ij = iK jK .
det (F )
Newtonian fluids. The components of the stress relate to the
components of the rate of deformation as
⎡ ∂v (x , t ) ∂v j (x , t ) ⎤
σ ij = η ⎢ i
+
⎥ − pδ ij ,
∂x i ⎥⎦
⎢⎣ ∂x j
where η is the viscosity. The material is assumed to be compressible:
∂vi (x , t )
=0.
∂x i
References
匡震邦, 非线性连续介质力学, 上海交通大学出版社, 2002. Written by the man
who taught me the subject in 1985 in Xian Jiaotong University.
黄筑平，连续介质力学基础，高等教育出版社， 2003.
G.A. Holzapfel, Nonlinear Solid Mechanics, Wiley, 2000.
C. Trusdell and W. Noll, The Non-linear Field Theories of Mechanics, 3rd edition,
Springer, 2004.
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