finite strain theory

In continuum mechanics, the finite strain theory—also called large strain theory, or large deformation theory—deals with deformations in which strains and/or rotations are large enough to invalidate assumptions inherent in infinitesimal strain theory. In this case, the undeformed and deformed configurations of the continuum are significantly different, requiring a clear distinction between them. This is commonly the case with elastomers, plastically-deforming materials and other fluids and biological soft tissue.

Displacement

The displacement of a body has two components: a rigid-body displacement and a deformation.
* A rigid-body displacement consists of a simultaneous translation (physics) and rotation of the body without changing its shape or size.
* Deformation implies the change in shape and/or size of the body from an initial or undeformed configuration $\kappa_0(\mathcal B)$ to a current or deformed configuration $\kappa_t(\mathcal B)$ (Figure 1).

A change in the configuration of a continuum body can be described by a displacement field. A ''displacement field'' is a vector field of all displacement vectors for all particles in the body, which relates the deformed configuration with the undeformed configuration. The distance between any two particles changes if and only if deformation has occurred. If displacement occurs without deformation, then it is a rigid-body displacement.

Material coordinates (Lagrangian description)

The displacement of particles indexed by variable may be expressed as follows. The vector joining the positions of a particle in the undeformed configuration $P_i$ and deformed configuration $p_i$ is called the displacement vector. Using $\mathbf$ in place of $P_i$ and $\mathbf$ in place of $p_i\,\!$, both of which are vectors from the origin of the coordinate system to each respective point, we have the Lagrangian description of the displacement vector:
$\mathbf u(\mathbf X,t) = u_i \mathbf e_i$
where $\mathbf e_i$ are the orthonormal unit vectors that define the basis of the spatial (lab-frame) coordinate system.

Expressed in terms of the material coordinates, i.e. $\mathbf u$ as a function of $\mathbf X$, the displacement field is:
$\mathbf u(\mathbf X, t) = \mathbf b(t)+\mathbf x(\mathbf X,t) - \mathbf X \qquad \text\qquad u_i = \alpha_ b_J + x_i - \alpha_ X_J$
where $\mathbf b(t)$ is the displacement vector representing rigid-body translation.

The partial derivative of the displacement vector with respect to the material coordinates yields the ''material displacement gradient tensor'' $\nabla_ \mathbf u\,\!$. Thus we have,
$\nabla_\mathbf u = \nabla_\mathbf x - \mathbf R = \mathbf F - \mathbf R \qquad \text \qquad \frac = \frac - \alpha_ = F_ - \alpha_$
where $\mathbf F$ is the ''deformation gradient tensor''.

Spatial coordinates (Eulerian description)

In the Eulerian description, the vector extending from a particle $P$ in the undeformed configuration to its location in the deformed configuration is called the displacement vector:
$\mathbf U(\mathbf x,t) = U_J\mathbf E_J$
where $\mathbf E_i$ are the unit vectors that define the basis of the material (body-frame) coordinate system.

Expressed in terms of spatial coordinates, i.e. $\mathbf U$ as a function of $\mathbf x$, the displacement field is:
$\mathbf U(\mathbf x, t) = \mathbf b(t) + \mathbf x - \mathbf X(\mathbf x,t) \qquad \text\qquad U_J = b_J + \alpha_ x_i - X_J$

The partial derivative of the displacement vector with respect to the spatial coordinates yields the ''spatial displacement gradient tensor'' $\nabla_ \mathbf U\,\!$. Thus we have,
$\nabla_\mathbf U = \mathbf R^ - \nabla_\mathbf X = \mathbf R^ -\mathbf F^ \qquad \text \qquad \frac = \alpha_ - \frac = \alpha_ - F^_ \,.$

Relationship between the material and spatial coordinate systems

$\alpha_$ are the direction cosines between the material and spatial coordinate systems with unit vectors $\mathbf E_J$ and $\mathbf e_i\,\!$, respectively. Thus
$\mathbf E_J \cdot \mathbf e_i = \alpha_ = \alpha_$

The relationship between $u_i$ and $U_J$ is then given by
$u_i=\alpha_U_J \qquad \text \qquad U_J=\alpha_ u_i$

Knowing that
$\mathbf e_i = \alpha_ \mathbf E_J$
then
$\mathbf u(\mathbf X, t) = u_i\mathbf e_i = u_i(\alpha_\mathbf E_J) = U_J \mathbf E_J = \mathbf U(\mathbf x, t)$

Combining the coordinate systems of deformed and undeformed configurations

It is common to superimpose the coordinate systems for the deformed and undeformed configurations, which results in $\mathbf b = 0\,\!$, and the direction cosines become Kronecker deltas, i.e.,
$\mathbf E_J \cdot \mathbf e_i = \delta_ = \delta_$

Thus in material (undeformed) coordinates, the displacement may be expressed as:
$\mathbf u(\mathbf X, t) = \mathbf x(\mathbf X,t) - \mathbf X \qquad \text\qquad u_i = x_i - \delta_ X_J$

And in spatial (deformed) coordinates, the displacement may be expressed as:
$\mathbf U(\mathbf x, t) = \mathbf x - \mathbf X(\mathbf x,t) \qquad \text\qquad U_J = \delta_ x_i - X_J$

Deformation gradient tensor

The deformation gradient tensor $\mathbf F(\mathbf X,t) = F_ \mathbf e_j \otimes \mathbf I_K$ is related to both the reference and current configuration, as seen by the unit vectors $\mathbf e_j$ and $\mathbf I_K\,\!$, therefore it is a ''two-point tensor''.

Due to the assumption of continuity of $\chi(\mathbf X,t)\,\!$, $\mathbf F$ has the inverse $\mathbf H = \mathbf F^\,\!$, where $\mathbf H$ is the ''spatial deformation gradient tensor''. Then, by the implicit function theorem, the Jacobian determinant $J(\mathbf X,t)$ must be nonsingular, i.e. $J(\mathbf X,t) = \det \mathbf F(\mathbf X,t) \neq 0$

The ''material deformation gradient tensor'' $\mathbf F(\mathbf X,t) = F_ \mathbf e_j\otimes\mathbf I_K$ is a second-order tensor that represents the gradient of the mapping function or functional relation $\chi(\mathbf X,t)\,\!$, which describes the motion of a continuum. The material deformation gradient tensor characterizes the local deformation at a material point with position vector $\mathbf X\,\!$, i.e., deformation at neighbouring points, by transforming (linear transformation) a material line element emanating from that point from the reference configuration to the current or deformed configuration, assuming continuity in the mapping function $\chi(\mathbf X,t)\,\!$, i.e. differentiable function of $\mathbf$ and time $t\,\!$, which implies that cracks and voids do not open or close during the deformation. Thus we have,
$\begin d\mathbf &= \frac \,d\mathbf \qquad &\text& \qquad dx_j =\frac\,dX_K \\ &= \nabla \chi(\mathbf X,t) \,d\mathbf \qquad &\text& \qquad dx_j =F_\,dX_K \,. \\ & = \mathbf F(\mathbf X,t) \,d\mathbf \end$

Relative displacement vector

Consider a particle or material point $P$ with position vector $\mathbf X = X_I \mathbf I_I$ in the undeformed configuration (Figure 2). After a displacement of the body, the new position of the particle indicated by $p$ in the new configuration is given by the vector position $\mathbf = x_i \mathbf e_i\,\!$. The coordinate systems for the undeformed and deformed configuration can be superimposed for convenience.

Consider now a material point $Q$ neighboring $P\,\!$, with position vector $\mathbf+ \Delta \mathbf = (X_I+\Delta X_I) \mathbf I_I\,\!$. In the deformed configuration this particle has a new position $q$ given by the position vector $\mathbf+ \Delta \mathbf\,\!$. Assuming that the line segments $\Delta X$ and $\Delta \mathbf x$ joining the particles $P$ and $Q$ in both the undeformed and deformed configuration, respectively, to be very small, then we can express them as $d\mathbf X$ and $d\mathbf x\,\!$. Thus from Figure 2 we have
$\begin \mathbf+ d\mathbf&= \mathbf+d\mathbf+\mathbf(\mathbf+d\mathbf) \\ d\mathbf &= \mathbf-\mathbf+d\mathbf+ \mathbf(\mathbf+d\mathbf) \\ &= d\mathbf+\mathbf(\mathbf+d\mathbf)- \mathbf(\mathbf) \\ &= d\mathbf+d\mathbf \\ \end$

where $\mathbf$ is the relative displacement vector, which represents the relative displacement of $Q$ with respect to $P$ in the deformed configuration.

Taylor approximation

For an infinitesimal element $d\mathbf X\,\!$, and assuming continuity on the displacement field, it is possible to use a Taylor series expansion around point $P\,\!$, neglecting higher-order terms, to approximate the components of the relative displacement vector for the neighboring particle $Q$ as
$\begin \mathbf(\mathbf+d\mathbf)&=\mathbf(\mathbf)+d\mathbf \quad & \text & \quad u_i^* = u_i+du_i \\ &\approx \mathbf(\mathbf)+\nabla_\mathbf u\cdot d\mathbf X \quad & \text & \quad u_i^* \approx u_i + \fracdX_J \,. \end$
Thus, the previous equation $d\mathbf x = d\mathbf + d\mathbf$ can be written as
$\begin d\mathbf x&=d\mathbf X+d\mathbf u \\ &=d\mathbf X+\nabla_\mathbf u\cdot d\mathbf X\\ &=\left(\mathbf I + \nabla_\mathbf u\right)d\mathbf X\\ &=\mathbf F d\mathbf X \end$

Time-derivative of the deformation gradient

Calculations that involve the time-dependent deformation of a body often require a time derivative of the deformation gradient to be calculated. A geometrically consistent definition of such a derivative requires an excursion into differential geometryA. Yavari, J.E. Marsden, and M. Ortiz
On spatial and material covariant balance laws in elasticity
Journal of Mathematical Physics, 47, 2006, 042903; pp. 1–53. but we avoid those issues in this article.

The time derivative of $\mathbf$ is
\dot = \frac = \frac \left frac\right= \frac\left frac\right= \frac\left mathbf(\mathbf, t)\right
where $\mathbf$ is the (material) velocity. The derivative on the right hand side represents a material velocity gradient. It is common to convert that into a spatial gradient by applying the chain rule for derivatives, i.e.,

\dot =
\frac\left mathbf(\mathbf, t)\right=
\frac\left mathbf(\mathbf(\mathbf, t),t)\right=
\left.\frac\left mathbf(\mathbf,t)\right_ \cdot
\frac
= \boldsymbol\cdot\mathbf

where $\boldsymbol$ is the spatial velocity gradient and where $\mathbf(\mathbf,t) = \mathbf(\mathbf,t)$ is the spatial (Eulerian) velocity at $\mathbf = \mathbf(\mathbf, t)$. If the spatial velocity gradient is constant in time, the above equation can be solved exactly to give
$\mathbf = e^$
assuming $\mathbf = \mathbf$ at $t = 0$. There are several methods of computing the exponential above.

Related quantities often used in continuum mechanics are the rate of deformation tensor and the spin tensor defined, respectively, as:
$\boldsymbol = \tfrac \left(\boldsymbol + \boldsymbol^T\right) \,,~~ \boldsymbol = \tfrac \left(\boldsymbol - \boldsymbol^T\right) \,.$
The rate of deformation tensor gives the rate of stretching of line elements while the spin tensor indicates the rate of rotation or vorticity of the motion.

The material time derivative of the inverse of the deformation gradient (keeping the reference configuration fixed) is often required in analyses that involve finite strains. This derivative is
$\frac \left(\mathbf^\right) = - \mathbf^ \cdot \dot \cdot \mathbf^ \,.$
The above relation can be verified by taking the material time derivative of $\mathbf^ \cdot d\mathbf = d\mathbf$ and noting that $\dot = 0$.

Transformation of a surface and volume element

To transform quantities that are defined with respect to areas in a deformed configuration to those relative to areas in a reference configuration, and vice versa, we use Nanson's relation, expressed as $da~\mathbf = J~dA ~\mathbf^ \cdot \mathbf$ where $da$ is an area of a region in the deformed configuration, $dA$ is the same area in the reference configuration, and $\mathbf$ is the outward normal to the area element in the current configuration while $\mathbf$ is the outward normal in the reference configuration, $\mathbf$ is the deformation gradient, and $J = \det\mathbf\,\!$.

The corresponding formula for the transformation of the volume element is $dv = J~dV$

Polar decomposition of the deformation gradient tensor

The deformation gradient $\mathbf\,\!$, like any invertible second-order tensor, can be decomposed, using the polar decomposition theorem, into a product of two second-order tensors (Truesdell and Noll, 1965): an orthogonal tensor and a positive definite symmetric tensor, i.e., $\mathbf = \mathbf \mathbf = \mathbf \mathbf$ where the tensor $\mathbf$ is a proper orthogonal tensor, i.e., $\mathbf R^ = \mathbf R^T$ and $\det \mathbf R = +1\,\!$, representing a rotation; the tensor $\mathbf$ is the ''right stretch tensor''; and $\mathbf$ the ''left stretch tensor''. The terms ''right'' and ''left'' means that they are to the right and left of the rotation tensor $\mathbf\,\!$, respectively. $\mathbf$ and $\mathbf$ are both positive definite, i.e. $\mathbf x \cdot \mathbf U \cdot \mathbf x > 0$ and $\mathbf x\cdot\mathbf V \cdot \mathbf x > 0$ for all non-zero $\mathbf x \in \R^3$, and symmetric tensors, i.e. $\mathbf U = \mathbf U^T$ and $\mathbf V = \mathbf V^T\,\!$, of second order.

This decomposition implies that the deformation of a line element $d\mathbf X$ in the undeformed configuration onto $d\mathbf x$ in the deformed configuration, i.e., $d\mathbf x = \mathbf F \,d\mathbf X\,\!$, may be obtained either by first stretching the element by $\mathbf U\,\!$, i.e. $d\mathbf x' = \mathbf U \,d\mathbf X\,\!$, followed by a rotation $\mathbf R\,\!$, i.e., $d\mathbf x' = \mathbf R \,d\mathbf x\,\!$; or equivalently, by applying a rigid rotation $\mathbf R$ first, i.e., $d\mathbf x' = \mathbf R \, d\mathbf X\,\!$, followed later by a stretching $\mathbf V\,\!$, i.e., $d\mathbf x' = \mathbf V \, d\mathbf x$ (See Figure 3).

Due to the orthogonality of $\mathbf R$
$\mathbf V = \mathbf R \cdot \mathbf U \cdot \mathbf R^T$
so that $\mathbf U$ and $\mathbf V$ have the same eigenvalues or ''principal stretches'', but different eigenvectors or ''principal directions'' $\mathbf_i$ and $\mathbf_i\,\!$, respectively. The principal directions are related by
$\mathbf_i = \mathbf \mathbf_i.$

This polar decomposition, which is unique as $\mathbf F$ is invertible with a positive determinant, is a corrolary of the singular-value decomposition.

Deformation tensors

Several rotation-independent deformation tensors are used in mechanics. In solid mechanics, the most popular of these are the right and left Cauchy–Green deformation tensors.

Since a pure rotation should not induce any strains in a deformable body, it is often convenient to use rotation-independent measures of deformation in continuum mechanics. As a rotation followed by its inverse rotation leads to no change ($\mathbf\mathbf^T=\mathbf^T\mathbf=\mathbf\,\!$) we can exclude the rotation by multiplying $\mathbf$ by its transpose.

The right Cauchy–Green deformation tensor

In 1839, George Green introduced a deformation tensor known as the ''right Cauchy–Green deformation tensor'' or ''Green's deformation tensor'', defined as:The IUPAC recommends that this tensor be called the Cauchy strain tensor.

$\mathbf C=\mathbf F^T\mathbf F=\mathbf U^2 \qquad \text \qquad C_=F_~F_ = \frac \frac .$

Physically, the Cauchy–Green tensor gives us the square of local change in distances due to deformation, i.e. $d\mathbf x^2=d\mathbf X\cdot\mathbf C \cdot d\mathbf X$

Invariants of $\mathbf$ are often used in the expressions for strain energy density functions. The most commonly used invariants are

\begin
I_1^C & := \text(\mathbf) = C_ = \lambda_1^2 + \lambda_2^2 + \lambda_3^2 \\
I_2^C & := \tfrac\left \text~\mathbf)^2 - \text(\mathbf^2) \right = \tfrac\left C_)^2 - C_C_\right= \lambda_1^2\lambda_2^2 + \lambda_2^2\lambda_3^2 + \lambda_3^2\lambda_1^2 \\
I_3^C & := \det(\mathbf) = J^2 = \lambda_1^2\lambda_2^2\lambda_3^2.
\end

where $J:=\det\mathbf$ is the determinant of the deformation gradient $\mathbf$ and $\lambda_i$ are stretch ratios for the unit fibers that are initially oriented along the eigenvector directions of the right (reference) stretch tensor (these are not generally aligned with the three axis of the coordinate systems).

The Finger deformation tensor

The IUPAC recommends that the inverse of the right Cauchy–Green deformation tensor (called the Cauchy tensor in that document), i. e., $\mathbf C^$, be called the Finger tensor. However, that nomenclature is not universally accepted in applied mechanics.

$\mathbf=\mathbf C^=\mathbf F^\mathbf F^ \qquad \text \qquad f_=\frac \frac$

The left Cauchy–Green or Finger deformation tensor

Reversing the order of multiplication in the formula for the right Green–Cauchy deformation tensor leads to the ''left Cauchy–Green deformation tensor'' which is defined as:
$\mathbf B = \mathbf F\mathbf F^T = \mathbf V^2 \qquad \text \qquad B_ = \frac \frac$

The left Cauchy–Green deformation tensor is often called the ''Finger deformation tensor'', named after Josef Finger (1894).The IUPAC recommends that this tensor be called the Green strain tensor.

Invariants of $\mathbf$ are also used in the expressions for strain energy density functions. The conventional invariants are defined as

\begin
I_1 & := \text(\mathbf) = B_ = \lambda_1^2 + \lambda_2^2 + \lambda_3^2\\
I_2 & := \tfrac\left \text~\mathbf)^2 - \text(\mathbf^2)\right = \tfrac\left(B_^2 - B_B_\right) = \lambda_1^2\lambda_2^2 + \lambda_2^2\lambda_3^2 + \lambda_3^2\lambda_1^2 \\
I_3 & := \det\mathbf = J^2 = \lambda_1^2\lambda_2^2\lambda_3^2
\end

where $J:=\det\mathbf$ is the determinant of the deformation gradient.

For compressible materials, a slightly different set of invariants is used:
$(\bar_1 := J^ I_1 ~;~~ \bar_2 := J^ I_2 ~;~~ J\neq 1) ~.$

The Cauchy deformation tensor

Earlier in 1828, Augustin-Louis Cauchy introduced a deformation tensor defined as the inverse of the left Cauchy–Green deformation tensor, $\mathbf B^\,\!$. This tensor has also been called the Piola tensor and the Finger tensor in the rheology and fluid dynamics literature.

$\mathbf=\mathbf B^=\mathbf F^\mathbf F^ \qquad \text \qquad c_=\frac \frac$

Spectral representation

If there are three distinct principal stretches $\lambda_i \,\!$, the spectral decompositions of $\mathbf$ and $\mathbf$ is given by

$\mathbf = \sum_^3 \lambda_i^2 \mathbf_i \otimes \mathbf_i \qquad \text \qquad \mathbf = \sum_^3 \lambda_i^2 \mathbf_i \otimes \mathbf_i$

Furthermore,

$\mathbf U = \sum_^3 \lambda_i \mathbf N_i \otimes \mathbf N_i ~;~~ \mathbf V = \sum_^3 \lambda_i \mathbf n_i \otimes \mathbf n_i$
$\mathbf R = \sum_^3 \mathbf n_i \otimes \mathbf N_i ~;~~ \mathbf F = \sum_^3 \lambda_i \mathbf n_i \otimes \mathbf N_i$

Observe that
$\mathbf = \mathbf~\mathbf~\mathbf^T = \sum_^3 \lambda_i~\mathbf~(\mathbf_i\otimes\mathbf_i)~\mathbf^T = \sum_^3 \lambda_i~(\mathbf~\mathbf_i)\otimes(\mathbf~\mathbf_i)$
Therefore, the uniqueness of the spectral decomposition also implies that $\mathbf_i = \mathbf~\mathbf_i \,\!$. The left stretch ($\mathbf\,\!$) is also called the ''spatial stretch tensor'' while the right stretch ($\mathbf\,\!$) is called the ''material stretch tensor''.

The effect of $\mathbf$ acting on $\mathbf_i$ is to stretch the vector by $\lambda_i$ and to rotate it to the new orientation $\mathbf_i\,\!$, i.e.,
$\mathbf~\mathbf_i = \lambda_i~(\mathbf~\mathbf_i) = \lambda_i~\mathbf_i$
In a similar vein,
$\mathbf^~\mathbf_i = \cfrac~\mathbf_i ~;~~ \mathbf^T~\mathbf_i = \lambda_i~\mathbf_i ~;~~ \mathbf^~\mathbf_i = \cfrac~\mathbf_i ~.$

Examples

; Uniaxial extension of an incompressible material
: This is the case where a specimen is stretched in 1-direction with a stretch ratio of $\mathbf\,\!$. If the volume remains constant, the contraction in the other two directions is such that $\mathbf$ or $\mathbf\,\!$. Then: $\mathbf=\begin \alpha & 0 & 0 \\ 0 & \alpha^ & 0 \\ 0 & 0 & \alpha^ \end$ $\mathbf = \mathbf = \begin \alpha^2 & 0 & 0 \\ 0 & \alpha^ & 0 \\ 0 & 0 & \alpha^ \end$
; Simple shear
:$\mathbf=\begin 1 & \gamma & 0 \\ 0 & 1 & 0 \\ 0 & 0 & 1 \end$ $\mathbf = \begin 1+\gamma^2 & \gamma & 0 \\ \gamma & 1 & 0 \\ 0 & 0 & 1 \end$ $\mathbf = \begin 1 & \gamma & 0 \\ \gamma & 1+\gamma^2 & 0 \\ 0 & 0 & 1 \end$
; Rigid body rotation
:$\mathbf = \begin \cos \theta & \sin \theta & 0 \\ - \sin \theta & \cos \theta & 0 \\ 0 & 0 & 1 \end$ $\mathbf = \mathbf = \begin 1 & 0 & 0 \\ 0 & 1 & 0 \\ 0 & 0 & 1 \end = \mathbf$

Derivatives of stretch

Derivatives of the stretch with respect to the right Cauchy–Green deformation tensor are used to derive the stress-strain relations of many solids, particularly hyperelastic materials. These derivatives are
$\cfrac = \cfrac~\mathbf_i\otimes\mathbf_i = \cfrac~\mathbf^T~(\mathbf_i\otimes\mathbf_i)~\mathbf ~;~~ i=1,2,3$
and follow from the observations that
$\mathbf:(\mathbf_i\otimes\mathbf_i) = \lambda_i^2 ~;~~~~\cfrac = \mathsf^ ~;~~~~ \mathsf^:(\mathbf_i\otimes\mathbf_i)=\mathbf_i\otimes\mathbf_i.$

Physical interpretation of deformation tensors

Let $\mathbf = X^i~\boldsymbol_i$ be a Cartesian coordinate system defined on the undeformed body and let $\mathbf = x^i~\boldsymbol_i$ be another system defined on the deformed body. Let a curve $\mathbf(s)$ in the undeformed body be parametrized using s \in ,1/math>. Its image in the deformed body is $\mathbf(\mathbf(s))$.

The undeformed length of the curve is given by
$l_X = \int_0^1 \left, \cfrac \~ds = \int_0^1 \sqrt~ds = \int_0^1 \sqrt~ds$
After deformation, the length becomes
$\begin l_x & = \int_0^1 \left, \cfrac \~ds = \int_0^1 \sqrt~ds = \int_0^1 \sqrt~ds \\ & = \int_0^1 \sqrt~ds \end$
Note that the right Cauchy–Green deformation tensor is defined as
$\boldsymbol := \boldsymbol^T\cdot\boldsymbol = \left(\cfrac\right)^T\cdot \cfrac$
Hence,
$l_x = \int_0^1 \sqrt~ds$
which indicates that changes in length are characterized by $\boldsymbol$.

Finite strain tensors

The concept of ''strain'' is used to evaluate how much a given displacement differs locally from a rigid body displacement. One of such strains for large deformations is the ''Lagrangian finite strain tensor'', also called the ''Green-Lagrangian strain tensor'' or ''Green – St-Venant strain tensor'', defined as

$\mathbf E=\frac(\mathbf C - \mathbf I)\qquad \text \qquad E_=\frac\left( \frac\frac-\delta_\right)$

or as a function of the displacement gradient tensor
\mathbf E =\frac\left (\nabla_\mathbf u)^T + \nabla_\mathbf u + (\nabla_\mathbf u)^T \cdot\nabla_\mathbf u\right/math>
or
$E_=\frac\left(\frac+\frac+\frac\frac\right)$

The Green-Lagrangian strain tensor is a measure of how much $\mathbf C$ differs from $\mathbf I\,\!$.

The ''Eulerian-Almansi finite strain tensor'', referenced to the deformed configuration, i.e. Eulerian description, is defined as

$\mathbf e=\frac(\mathbf I - \mathbf c)=\frac(\mathbf I - \mathbf B ^) \qquad \text \qquad e_ = \frac \left(\delta_ - \frac \frac\right)$

or as a function of the displacement gradients we have
$e_ = \frac \left(\frac + \frac - \frac \frac\right)$

d\mathbf=\mathbf F^ \, d\mathbf=\mathbf \,d\mathbf \qquad \text \qquad dX_M=\frac\, dx_n
where $\frac$ are the components of the ''spatial deformation gradient tensor'', $\mathbf\,\!$. Thus we have

$\begin d\mathbf^2 &= d\mathbf X \cdot d\mathbf X \\ &= \mathbf F^ \cdot d\mathbf x \cdot \mathbf F^ \cdot d\mathbf x \\ &= d\mathbf x \cdot \mathbf F^\mathbf F^ \cdot d\mathbf x \\ &= d\mathbf x\cdot\mathbf c\cdot d\mathbf x \end \qquad \text \qquad \begin (dX)^2&=dX_M\,dX_M \\ &= \frac\frac\,dx_r\,dx_s \\ &= c_\,dx_r\,dx_s \\ \end$
where the second order tensor $c_$ is called ''Cauchy's deformation tensor'', $\mathbf c=\mathbf F^\mathbf F^\,\!$. Then we have,

$\begin d\mathbf^2 - d\mathbf^2 &= d\mathbf x\cdot d\mathbf x-d\mathbf x\cdot\mathbf c\cdot d\mathbf x \\ &=d\mathbf x\cdot (\mathbf I - \mathbf c)\cdot d\mathbf x \\ &= d\mathbf x \cdot 2\mathbf e \cdot d\mathbf x \\ \end$
or
$\begin (dx)^2 - (dX)^2 &= dx_j\,dx_j-\frac\frac\,dx_r\,dx_s \\ &= \left(\delta_ - \frac\frac \right)\,dx_r\,dx_s \\ &=2e_\,dx_r\,dx_s \end$

where $e_\,\!$, are the components of a second-order tensor called the ''Eulerian-Almansi finite strain tensor'',
$\mathbf e=\frac(\mathbf I - \mathbf c) \qquad \text \qquad e_=\frac\left(\delta_ - \frac\frac \right)$

Both the Lagrangian and Eulerian finite strain tensors can be conveniently expressed in terms of the ''displacement gradient tensor''. For the Lagrangian strain tensor, first we differentiate the displacement vector $\mathbf u(\mathbf X, t)$ with respect to the material coordinates $X_M$ to obtain the ''material displacement gradient tensor'', $\nabla_\mathbf u$

$\begin \mathbf u(\mathbf X,t) &= \mathbf x(\mathbf X,t) - \mathbf X \\ \nabla_\mathbf u &= \mathbf F - \mathbf I \\ \mathbf F &= \nabla_\mathbf u + \mathbf I \\ \end \qquad \text \qquad \begin u_i& = x_i-\delta_X_J \\ \delta_U_J &= x_i-\delta_X_J \\ x_i&=\delta_\left(U_J+X_J\right) \\ \frac&=\delta_\left(\frac+\delta_\right) \\ \end$

Replacing this equation into the expression for the Lagrangian finite strain tensor we have
\begin
\mathbf E &= \frac\left(\mathbf F^T\mathbf F-\mathbf I\right) \\
&=\frac\left \left\\left( \nabla_\mathbf u+\mathbf I\right)-\mathbf I\right\\
&=\frac\left (\nabla_\mathbf u)^T + \nabla_\mathbf u + (\nabla_\mathbf u)^T \cdot\nabla_\mathbf u\right\\
\end
or
\begin
E_&=\frac\left( \frac \frac - \delta_\right) \\
&=\frac \left delta_\left(\frac+\delta_\right)\delta_\left(\frac+\delta_\right)-\delta_\right\\
&=\frac\left delta_\left(\frac+\delta_\right)\left(\frac+\delta_\right)-\delta_\right\\
&=\frac\left left(\frac+\delta_\right)\left(\frac+\delta_\right)-\delta_\right\\
&=\frac\left(\frac +\frac +\frac \frac\right)
\end

Similarly, the Eulerian-Almansi finite strain tensor can be expressed as

$e_ = \frac \left(\frac +\frac - \frac \frac\right)$

Seth–Hill family of generalized strain tensors

B. R. Seth from the Indian Institute of Technology Kharagpur was the first to show that the Green and Almansi strain tensors are special cases of a more general strain measure. The idea was further expanded upon by Rodney Hill in 1968. The Seth–Hill family of strain measures (also called Doyle-Ericksen tensors)T.C. Doyle and J.L. Eriksen (1956). "Non-linear elasticity." ''Advances in Applied Mechanics'' 4, 53–115. can be expressed as

\mathbf E_=\frac(\mathbf U^- \mathbf I) = \frac\left mathbf^ - \mathbf\right/math>

For different values of $m$ we have:
* Green-Lagrangian strain tensor $\mathbf E_ = \frac (\mathbf U^- \mathbf I) = \frac (\mathbf-\mathbf)$
* Biot strain tensor $\mathbf E_ = (\mathbf U - \mathbf I) = \mathbf^-\mathbf$
* Logarithmic strain, Natural strain, True strain, or Hencky strain $\mathbf E_ = \ln \mathbf U = \frac\,\ln\mathbf$
* Almansi strain \mathbf_ = \frac\left mathbf-\mathbf^\right/math>
The second-order approximation of these tensors is
$\mathbf_ = \boldsymbol + (\nabla\mathbf)^T\cdot\nabla\mathbf - (1 - m) \boldsymbol^T\cdot\boldsymbol$
where $\boldsymbol$ is the infinitesimal strain tensor.

Many other different definitions of tensors $\mathbf$ are admissible, provided that they all satisfy the conditions that:Z.P. Bažant and L. Cedolin (1991). ''Stability of Structures. Elastic, Inelastic, Fracture and Damage Theories.'' Oxford Univ. Press, New York (2nd ed. Dover Publ., New York 2003; 3rd ed., World Scientific 2010).
* $\mathbf$ vanishes for all rigid-body motions
* the dependence of $\mathbf$ on the displacement gradient tensor $\nabla\mathbf$ is continuous, continuously differentiable and monotonic
* it is also desired that $\mathbf$ reduces to the infinitesimal strain tensor $\boldsymbol$ as the norm $, \nabla\mathbf, \to 0$

An example is the set of tensors
$\mathbf^ = \left(^n - ^\right)/2n$
which do not belong to the Seth–Hill class, but have the same 2nd-order approximation as the Seth–Hill measures at $m=0$ for any value of $n$.Z.P. Bažant (1998).
Easy-to-compute tensors with symmetric inverse approximating Hencky finite strain and its rate
" ''Journal of Materials of Technology ASME'', 120 (April), 131–136.

Stretch ratio

The stretch ratio is a measure of the extensional or normal strain of a differential line element, which can be defined at either the undeformed configuration or the deformed configuration.

The stretch ratio for the differential element $d\mathbf X = dX \mathbf N$ (Figure) in the direction of the unit vector $\mathbf N$ at the material point $P\,\!$, in the undeformed configuration, is defined as
$\Lambda_ = \frac$
where $dx$ is the deformed magnitude of the differential element $d\mathbf X\,\!$.

Similarly, the stretch ratio for the differential element $d\mathbf x = dx\mathbf n$ (Figure), in the direction of the unit vector $\mathbf n$ at the material point $p\,\!$, in the deformed configuration, is defined as
$\frac = \frac.$

The normal strain $e_$ in any direction $\mathbf N$ can be expressed as a function of the stretch ratio,
$e_= \frac=\Lambda_- 1.$

This equation implies that the normal strain is zero, i.e. no deformation, when the stretch is equal to unity. Some materials, such as elastometers can sustain stretch ratios of 3 or 4 before they fail, whereas traditional engineering materials, such as concrete or steel, fail at much lower stretch ratios, perhaps of the order of 1.1 (reference?)

Physical interpretation of the finite strain tensor

The diagonal components $E_$ of the Lagrangian finite strain tensor are related to the normal strain, e.g.

$E_=e_+\frac e_^2$

where $e_$ is the normal strain or engineering strain in the direction $\mathbf I_1\,\!$.

The off-diagonal components $E_$ of the Lagrangian finite strain tensor are related to shear strain, e.g.

$E_=\frac\sqrt\sqrt\sin\phi_$

where $\phi_$ is the change in the angle between two line elements that were originally perpendicular with directions $\mathbf I_1$ and $\mathbf I_2\,\!$, respectively.

Under certain circumstances, i.e. small displacements and small displacement rates, the components of the Lagrangian finite strain tensor may be approximated by the components of the infinitesimal strain tensor

= \frac

The square of the stretch ratio is defined as
$\Lambda_^2=\left (\frac\right )^2$

Knowing that
$(dx)^2=C_dX_KdX_L$
we have
$\Lambda_^2 = C_ N_K N_L$
where $N_K$ and $N_L$ are unit vectors.

The normal strain or engineering strain $e_$ in any direction $\mathbf N$ can be expressed as a function of the stretch ratio,

$e_=\frac=\Lambda_-1$

Thus, the normal strain in the direction $\mathbf I_1$ at the material point $P$ may be expressed in terms of the stretch ratio as

$\begin e_=\frac&=\Lambda_-1\\ &=\sqrt -1=\sqrt-1\\ &=\sqrt-1 \end$

solving for $E_$ we have

$\begin 2E_&= \frac \\ E_&= \left(\frac\right)+ \frac \left(\frac\right)^2 \\ &=e_+\frace_^2 \end$

The ''shear strain'', or change in angle between two line elements $d\mathbf X_1$ and $d\mathbf X_2$ initially perpendicular, and oriented in the principal directions $\mathbf I_1$ and $\mathbf I_2\,\!$, respectively, can also be expressed as a function of the stretch ratio. From the dot product between the deformed lines $d\mathbf x_1$ and $d\mathbf x_2$ we have

$\begin d\mathbf x_1 \cdot d\mathbf x_2 &=dx_1 dx_2 \cos\theta_ \\ \mathbf F \cdot d\mathbf X_1\cdot \mathbf F\cdot d\mathbf X_2&= \sqrt \cdot \sqrt \cos\theta_ \\ \frac &=\frac \cos\theta_\\ \mathbf I_1 \cdot \mathbf C \cdot \mathbf I_2&= \Lambda_\Lambda_\cos\theta_ \end$

where $\theta_$ is the angle between the lines $d\mathbf x_1$ and $d\mathbf x_2$ in the deformed configuration. Defining $\phi_$ as the shear strain or reduction in the angle between two line elements that were originally perpendicular, we have

$\phi_=\frac-\theta_$
thus,
$\cos\theta_=\sin\phi_$
then
$\mathbf I_1 \cdot \mathbf C \cdot \mathbf I_2= \Lambda_ \Lambda_\sin\phi_$

or

$\begin C_&=\sqrt\sqrt\sin\phi_\\ 2E_+\delta_&=\sqrt\sqrt\sin\phi_\\ E_&=\frac\sqrt\sqrt\sin\phi_ \end$

Deformation tensors in convected curvilinear coordinates

A representation of deformation tensors in curvilinear coordinates is useful for many problems in continuum mechanics such as nonlinear shell theories and large plastic deformations. Let $\mathbf = \mathbf(\xi^1,\xi^2,\xi^3)$ denote the function by which a position vector in space is constructed from coordinates $(\xi^1,\xi^2,\xi^3)$. The coordinates are said to be "convected" if they correspond to a one-to-one mapping to and from Lagrangian particles in a continuum body. If the coordinate grid is "painted" on the body in its initial configuration, then this grid will deform and flow with the motion of material to remain painted on the same material particles in the deformed configuration so that grid lines intersect at the same material particle in either configuration. The tangent vector to the deformed coordinate grid line curve $\xi^i$ at $\mathbf$ is given by
$\mathbf_i = \frac$
The three tangent vectors at $\mathbf$ form a local basis. These vectors are related the reciprocal basis vectors by
$\mathbf_i\cdot\mathbf^j = \delta_i^j$

Let us define a second-order tensor field $\boldsymbol$ (also called the metric tensor) with components
$g_ := \frac\cdot\frac = \mathbf_i\cdot\mathbf_j$
The Christoffel symbols of the first kind can be expressed as

\Gamma_
= \tfrac \mathbf_i\cdot\mathbf_k)_ + (\mathbf_j\cdot\mathbf_k)_ - (\mathbf_i\cdot\mathbf_j)_

To see how the Christoffel symbols are related to the Right Cauchy–Green deformation tensor let us similarly define two bases, the already mentioned one that is tangent to deformed grid lines and another that is tangent to the undeformed grid lines. Namely,
$\mathbf_i := \frac ~;~~ \mathbf_i\cdot\mathbf^j = \delta_i^j ~;~~ \mathbf_i := \frac ~;~~ \mathbf_i\cdot\mathbf^j = \delta_i^j$

The deformation gradient in curvilinear coordinates

Using the definition of the gradient of a vector field in curvilinear coordinates, the deformation gradient can be written as
$\boldsymbol = \boldsymbol_\mathbf = \frac\otimes\mathbf^i = \mathbf_i\otimes\mathbf^i$

The right Cauchy–Green tensor in curvilinear coordinates

The right Cauchy–Green deformation tensor is given by
$\boldsymbol = \boldsymbol^T\cdot\boldsymbol = (\mathbf^i\otimes\mathbf_i)\cdot(\mathbf_j\otimes\mathbf^j) = (\mathbf_i\cdot\mathbf_j)(\mathbf^i\otimes\mathbf^j)$
If we express $\boldsymbol$ in terms of components with respect to the basis we have
$\boldsymbol = C_~\mathbf^i\otimes\mathbf^j$
Therefore,
$C_ = \mathbf_i\cdot\mathbf_j = g_$

and the corresponding Christoffel symbol of the first kind may be written in the following form.

\Gamma_
= \tfrac _ + C_ - C_ = \tfrac \mathbf_i\cdot\boldsymbol\cdot\mathbf_k)_ + (\mathbf_j\cdot\boldsymbol\cdot\mathbf_k)_ - (\mathbf_i\cdot\boldsymbol\cdot\mathbf_j)_

Some relations between deformation measures and Christoffel symbols

Consider a one-to-one mapping from $\mathbf = \$ to $\mathbf = \$ and let us assume that there exist two positive-definite, symmetric second-order tensor fields $\boldsymbol$ and $\boldsymbol$ that satisfy
$G_ = \frac~\frac~g_$
Then,
$\frac = \left(\frac~\frac + \frac~\frac\right)~g_ + \frac~\frac~\frac$
Noting that
$\frac = \frac~\frac$
and $g_ = g_$ we have
$\begin \frac & = \left(\frac~\frac + \frac~\frac\right)~g_ + \frac~\frac~\frac~\frac \\ \frac & = \left(\frac~\frac + \frac~\frac\right)~g_ + \frac~\frac~\frac~\frac \\ \frac & = \left(\frac~\frac + \frac~\frac\right)~g_ + \frac~\frac~\frac~\frac \end$
Define
$\begin _\Gamma_ & := \frac\left(\frac + \frac - \frac\right) \\ _\Gamma_ & := \frac\left(\frac + \frac - \frac\right) \\ \end$
Hence
$_\Gamma_ = \frac~\frac~\frac \,_\Gamma_ + \frac~\frac~g_$
Define
^= _ ~;~~ ^= _
Then
$G^ = \frac~\frac~g^$
Define the Christoffel symbols of the second kind as
$_\Gamma^m_ := G^ \,_\Gamma_ ~;~~ _\Gamma^\nu_ := g^ \,_\Gamma_$
Then
$\begin _\Gamma^m_ & = G^~\frac~\frac~\frac \,_\Gamma_ + G^~\frac~\frac~g_ \\ & = \frac~\frac~g^~\frac~\frac~\frac \,_\Gamma_ + \frac~\frac~g^~\frac~\frac~g_ \\ & = \frac~\delta^\gamma_\rho~g^~\frac~\frac \,_\Gamma_ + \frac~\delta^\beta_\rho~g^~\frac~g_ \\ & = \frac~g^~\frac~\frac \,_\Gamma_ + \frac~g^~\frac~g_ \\ & = \frac~\frac~\frac \,_\Gamma^\nu_ + \frac~\delta^_~\frac \end$
Therefore,
$_\Gamma^m_ = \frac~\frac~\frac \,_\Gamma^\nu_ + \frac~\frac$
The invertibility of the mapping implies that
$\begin \frac\,_\Gamma^m_ & = \frac~\frac~\frac~\frac \,_\Gamma^\nu_ + \frac~\frac~\frac \\ & = \delta^\mu_\nu~\frac~\frac \,_\Gamma^\nu_ + \delta^\mu_\alpha~\frac \\ & = \frac~\frac \,_\Gamma^\mu_ + \frac \end$
We can also formulate a similar result in terms of derivatives with respect to $x$. Therefore,
$\begin \frac & = \frac\,_\Gamma^m_ - \frac~\frac \,_\Gamma^\mu_ \\ \frac & = \frac\,_\Gamma^\mu_ - \frac~\frac \,_\Gamma^m_ \end$

Compatibility conditions

The problem of compatibility in continuum mechanics involves the determination of allowable single-valued continuous fields on bodies. These allowable conditions leave the body without unphysical gaps or overlaps after a deformation. Most such conditions apply to simply-connected bodies. Additional conditions are required for the internal boundaries of multiply connected bodies.

Compatibility of the deformation gradient

The necessary and sufficient conditions for the existence of a compatible $\boldsymbol$ field over a simply connected body are
$\boldsymbol\times\boldsymbol = \boldsymbol$

Compatibility of the right Cauchy–Green deformation tensor

The necessary and sufficient conditions for the existence of a compatible $\boldsymbol$ field over a simply connected body are

R^\gamma_ :=
\frac ,_\Gamma^\gamma_-
\frac ,_\Gamma^\gamma_+
\,_\Gamma^\gamma_\,_\Gamma^\mu_ -
\,_\Gamma^\gamma_\,_\Gamma^\mu_ = 0

We can show these are the mixed components of the Riemann–Christoffel curvature tensor. Therefore, the necessary conditions for $\boldsymbol$-compatibility are that the Riemann–Christoffel curvature of the deformation is zero.

Compatibility of the left Cauchy–Green deformation tensor

No general sufficiency conditions are known for the left Cauchy–Green deformation tensor in three-dimensions. Compatibility conditions for two-dimensional $\boldsymbol$ fields have been found by Janet Blume.

See also

* Infinitesimal strain
* Compatibility (mechanics)
* Curvilinear coordinates
* Piola–Kirchhoff stress tensor, the stress tensor for finite deformations.
* Stress measures
* Strain partitioning

References

Further reading

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*{{Cite book
, last = Rees , first = David
, title = Basic Engineering Plasticity – An Introduction with Engineering and Manufacturing Applications
, publisher = Butterworth-Heinemann
, year = 2006
, url = https://books.google.com/books?id=4KWbmn_1hcYC
, isbn = 0-7506-8025-3

External links

Prof. Amit Acharya's notes on compatibility on iMechanica

Tensors
Continuum mechanics
Elasticity (physics)
Non-Newtonian fluids
Solid mechanics