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# Mode-I and Mode-II Crack Tip Fields in Implicit Gradient Elasticity Based on Laplacians of Stress and Strain. Part I: Governing Equations

By Carsten Broese, Jan Frischmann and Charalampos Tsakmakis

Submitted: July 8th 2020Reviewed: July 29th 2020Published: September 21st 2020

DOI: 10.5772/intechopen.93506

## Abstract

Models of implicit gradient elasticity based on Laplacians of stress and strain can be established in analogy to the models of linear viscoelastic solids. The most simple implicit gradient elasticity model including both, the Laplacian of stress and the Laplacian of strain, is the counterpart of the three-parameter viscoelastic solid. The main investigations in Parts I, II, and III concern the “three-parameter gradient elasticity model” and focus on the near-tip fields of Mode-I and Mode-II crack problems. It is proved that, for the boundary and symmetry conditions assumed in the present work, the model does not avoid the well-known singularities of classical elasticity. Nevertheless, there are significant differences in the form of the asymptotic solutions in comparison to the classical elasticity. These differences are discussed in detail on the basis of closed-form analytical solutions. Part I provides the governing equations and the required boundary and symmetry conditions for the considered crack problems.

### Keywords

• Laplacians of stress
• Laplacians of strain
• micromorphic and micro-strain elasticity
• plane strain state

## 1. Introduction

The most simple constitutive law in explicit gradient elasticity is the model with equation:

Σij=Cijmnεmnc2CijmnΔεmnKGModel.E1

Here, Σ=ΣTis the Cauchy stress tensor, εis the strain tensor, Cis the isotropic elasticity tensor, Δis the Laplacian operator, and c2is a material parameter, with c2denoting an internal material length. The components in Eq. (1) are referred to a Cartesian coordinate system. It seems that the constitutive law (1) has been introduced for the first time by Altan and Aifantis [1]. These authors (cf. also Georgiadis [2]) showed that the constitutive Eq. (1) leads to regular strain solutions at the crack tip of Mode-III crack problems. However, the stress field remains singular at the crack tip as in the case of classical elasticity. Moreover, Altan and Aifantis [1], as well as Georgiadis [2], presented an appropriate isotropic energy function for the mechanical model in Eq. (1) in the context of Mindlins gradient elasticity theory (see Mindlin [3] as well as Mindlin and Eshel [4]). An alternative approach to this model has been proposed in Broese et al. [5], where an analogy between gradient elasticity models and linear viscoelastic solids is established. According to this analogy, Eq. (1) is regarded as the gradient elasticity counterpart of the Kelvin viscoelastic solid. The short hand notation “KG-Model” in Eq. (1) stands for “Kelvin-Gradient-Elasticity-Model.”

Now, the question arises, if a gradient elasticity model including both, the Laplacian of stress and the Laplacian of strain, could remove both, the singularities of stress and the singularities of strain at the crack tip (cf. Gutkin and Aifantis [6]). The most simple generalization of Eq. (1), including the Laplacians of stress and strain, reads as follows:

Σijc1ΔΣij=Cijmnεmnc2CijmnΔεmn3PGModel,E2

where the same notation as in Eq. (1) applies and c1is a further internal material length. To our knowledge, model (2) has been introduced for the first time by Gutkin and Aifantis [6]. These authors proposed the gradient elasticity law (2) ad hoc in an attempt to eliminate the singularities of stress and strain of defects. Equations of the form (2) are known as models of implicit gradient elasticity (see Askes and Gutiérrez [7]).

Broese et al. [5] proved that Eq. (2) can be derived as a particular case of Mindlins micro-structured elasticity, which arises whenever the micro-deformation of the micromorphic continuum is supposed to be a symmetric tensor. Because the micro-structured elastic continuum of Mindlin and the micromorphic elastic continuum of Eringen (see, e.g., Eringen and Suhubi [8] and Eringen [9]) are essentially equivalent to each other, in the present work we will call both as micromorphic continua. According to Forest and Sievert [10], the resulting micromorphic theory is named micro-strain theory. It is shown in Broese et al. [5] that, in the context of micro-strain elasticity, the 3-PG-Model (2) can be derived as a combination of elasticity constitutive laws and the equilibrium equation for the so-called double stress.

On the other hand, Broese et al. [5] showed that Eq. (2) can be established alternatively by supposing the continuum to be classical, i.e., exhibiting only classical displacement degrees of freedom, but in the framework of the non-conventional thermodynamics proposed in Alber et al. [11]. To be more specific, the micro-deformation variable of the micro-strain approach has to be viewed as an internal state variable analogous to the inelastic strain in linear viscoelasticity. Eq. (2) then turns out to be a constitutive law, which is the counterpart in gradient elasticity of the three-parameter viscoelastic solid. The short hand notation “3-PG-Model” stands for “3-Parameter-Gradient-Elasticity-Model.” A general analogy to the constitutive laws describing viscoelastic solids can be established by using a nonstandard spring in gradient elasticity corresponding to the dashpot element in linear viscoelasticity and the Laplacian operator Δin place of the ordinary time derivative in the evolution laws of dashpot elements. Using virtual power balance arguments, Broese et al. [5] derived the same boundary conditions along the lines of the second approach as in the micro-strain approach. But now the boundary conditions have to be understood as constitutive boundary conditions, analogous to the constitutive initial conditions in viscoelasticity.

Because all resulting governing equations and boundary conditions in the two approaches are equal to each other, we shall proceed further by regarding the 3-PG-Model as a particular case of the micro-strain elasticity. The present work (Parts I, II, and III) is concerned with the near-tip fields predicted by the 3-PG-Model for Mode-I and Mode-II types of crack problems. Unlike statements made somewhere else (see Part II), we prove that, for the assumptions made here, the 3-PG-Model does not eliminate the well-known singularities of classical elasticity. Nevertheless, compared with the form of asymptotic solutions in classical elasticity, there are interesting new aspects, which are discussed in detail in Part IIon the basis of closed-form analytical solutions. Part Iprovides the governing equations and the required boundary and symmetry conditions in order to establish the analytical solutions.

## 2. Preliminaries: notation

Throughout the paper, we largely use the same notation as in Mindlin [3] and Mindlin and Eshel [4], in order to facilitate the comparison with these works. The deformations are assumed to be small, so we do not distinguish, as usually done, between reference and actual configuration. All indices will have the range of integers (1,2,3), while summation over repeated indices is implied. Explicit reference to space and time variables, upon which a function may depend, will be dropped in most part of the paper. Also, we shall not distinguish between functions and their values. However, if necessary, we shall give explicitly the set of variables which the function depends on.

Let Bbe a material body which may be identified by the position vectors x=xiei, with respect to a Cartesian coordinate system xiinducing the orthonormal basis ei. The body Boccupies the space Vin the three-dimensional Euclidean space we deal with. We indicate by nthe outward unit normal vector to the surface Vbounding the space V. Small Latin indices will be used in conjunction with Cartesian coordinates and related components. If fis a function of the Cartesian coordinates xi, then we shall use the notations for partial derivatives as follows:

iffxi,ijf2fxixj.E3

Let =ieibe the nabla operator and abe some vector or higher order tensor. The gradient, the divergence, and the Laplacian of aare defined, respectively, by gradaaa, divaa, and Δa=divgrada, where and are the scalar and the tensorial products between two vectors. It is helpful to use notations for components of the form aij=aij. Thus, if Aijand Aijkare the Cartesian components of a second-order tensor Aand a third-order tensor A, then, with respect to the Cartesian basis ei, we have the following equations:

Aijk=iAjk,E4
divAi=jAji,E5
ΔAij=kkAij,E6
divAij=kAkij.E7

We denote by Cthe fourth-order isotropic elasticity tensor with Cartesian components as follows:

Cijmn=λδijδmn+μδimδjn+δinδjm,E8

where λand μare the Lamé constants and δijis the Kronecker delta. For some calculations, it will be convenient to use the Young’s modulus Eand the Poisson ratio ν,

ν=λ2λ+μ,E=2μ1+ν.E9

Since Csatisfies the symmetry properties

Cijmn=Cjimn=Cmnij=Cijnm,E10

we have for every second-order tensor A, that

CijmnAmn=AmnCmnij.E11

For any tensor awith components aijkp, we write aijkpfor its symmetric part with respect to the indices jand k. Thus, if Asis the symmetric part of a second-order tensor A, then Aij=Aijs. Corresponding notations apply with regard to components related to curvilinear coordinate systems. Of particular interest for our work are cylindrical coordinates rφz. We find it convenient to use Greek indices α,β,to indicate both, physical components with respect to cylindrical coordinates and cylindrical coordinates itself. Thus, e.g., we write Aαβfor the physical components of the second-order tensor Aand denote by Aαβthe matrix of components,

Aαβ=ArrAArzAφrAφφAφzAzrAAzz.E12

Similar notations hold for any tensor of arbitrary order. The summation convention applies in analogous manner, e.g., we have Aαα=Arr+Aφφ+Azz. Because cylindrical coordinate systems are orthogonal, the algebraic operations between the corresponding physical components of tensors are identical in form to those with respect to Cartesian components. Moreover, the physical components of isotropic tensors are identical to their Cartesian components, e.g., the physical components of the isotropic elasticity tensor Cin Eq. (8) are given as follows:

Cαβγζ=λδαβδγζ+μδαγδβζ+δαζδβγ.E13

The physical components with respect to cylindrical coordinates of A,ΔAand divAare calculated in A. For partial derivatives of a function fwith respect to cylindrical coordinates, we use notations, in analogy to Eq. (3), of the forms

rffr,φffφ,zffz,E14
rrf2frr,.E15

## 3. Governing equations for the 3-PG-Model

This section provides a short overview about the 3-PG-Model in a form which is adequate for developing analytical solutions.

### 3.1 The 3-PG-Model as particular case of micro-strain elasticity

Assume the material body to be a micromorphic continuum. Besides the classical kinematical degrees of freedom, micromorphic continua are characterized by additional degrees of freedom due to the deformations of the micro-continua, which are assumed to be attached at every point of the macro-continuum (see Mindlin [3] and Broese et al. [5]). Therefore, in the micromorphic continuum theory, a nonclassical (double) stress and a nonclassical stress power are introduced in addition to the classical ones, but otherwise the theory is formulated in the framework of classical thermodynamics.

Let Ψbe the micro-deformation tensor of a micromorphic continuum, ube the macro-displacement vector, and εbe the macro-strain tensor,

εijεij12iuj+jui.E16

All component representations in Section 3 are referred to the Cartesian coordinate system xi. Assume Ψand the so-called relative deformation γto be symmetric,

ΨijΨij,γijγijεijΨij.E17

This means that Ψand γare strain tensors and that the components of the so-called micro-deformation gradient k,

kijkΨijk=iΨjk,E18

exhibit the symmetry property

kijkkijk.E19

Following Forest and Sievert [10], we denote a micromorphic elasticity theory based on Eqs. (16)(18) as micro-strain elasticity.

According to Broese et al. [5], the 3-PG-model can be established as a particular case of the micro-strain elasticity by assuming the existence of a free energy (per unit macro-volume) ψof the form:

ψ=ψεγk=12εijCijmnεmn+12c2c1c1γijCijmnγmn+12c2c1kijkCjkmnkimn.E20

The components Cijmnare defined in Eq. (8) and c1as well as c2are scalar parameters constrained to c2>c1>0with c1and c2denoting internal material lengths as noted in Section 1. The Cauchy stress tensor Σis then given by (cf. Broese et al. [5]):

ΣijΣij=τij+σij=c2c1Cijmnεmnc2c1c1CijmnΨmn,E21

where

τijτij=ψεij=Cijmnεmn,E22
σijσij=ψγij=c2c1c1CijmnεmnCijmnΨmn.E23

Further, there exists a double stress μwhich satisfies the potential relation

μijkμijk=ψkijk=c2c1iΨmnCmnjk.E24

For static problems, the classical and nonclassical stresses have to satisfy corresponding equilibrium equations. In the absence of body forces and body double forces, these are (see Mindlin [3] or Broese et al. [5])

jΣji=0,E25
kμkij+σij=0.E26

The concomitant classical and nonclassical boundary conditions are as follows:

Either Pi=njΣji or ui class.bound.cond.,E27
and either Tij=nkμkij or Ψij nonclass.bound.cond.,E28

have to be prescribed on the boundary V.

The 3-PG-Model can be obtained from the above equations by first inserting Eq. (24) into Eq. (26), as follows:

σij=kμkij=c2c1kkΨmnCmnij=c2c1CijmnΔΨmn.E29

Then take the Laplacian of Eq. (21), as follows:

ΔΣij=c2c1CijmnΔεmnc2c1c1CijmnΔΨmn,E30

and use Eq. (21) as well as Eq. (22) in Eq. (29), as follows:

c2c1CijmnΔΨmn=σij=ΣijCijmnεmn.E31

The latter together with Eq. (30) yield the following equation:

Σijc1ΔΣij=Cijmnεmnc2CijmnΔεmn,E32

which is nothing but the 3-PG-Model (2).

#### 3.1.1 A useful equation for Ψ

For later reference, we derive a useful equation for the strain Ψ. When seeking analytical solutions, there are two possibilities, either to find solutions in terms of Ψor in terms of μ. In the first case, μis eliminated at the cost of a higher order partial differential equation, but no compatibility conditions for Ψare needed. To be more specific, assuming C1to exist, we infer from Eqs. (23) and (29) that

εij=Ψijc1ΔΨij.E33

Further, from Eq. (21), we get the following equation:

εij=c1c2C1ijmnΣmn+c2c1c2Ψij.E34

By combining the last two equations, we gain the useful relation as follows:

Ψijc2ΔΨijC1ijmnΣmn=0.E35

For given Σ, this is a (Helmholtz) partial differential equation for the components of Ψ.

## 4. Mode-I and mode-II crack problems

In Part II, we consider Mode-I and Mode-II loading conditions for a sharp crack in the context of plane strain problems and employ cylindrical coordinates rφzas indicated in Figure 1. The aim of this section is to set up all relevant equations which are needed in Part II.

### 4.1 Kinematics

Plane strain state of micro-strain continua in equilibrium is characterized by the assumptions that

uα=uruφ0,εαβ=εrrε0εεφφ0000,E36
Ψαβ=ΨrrΨ0ΨΨφφ0000,E37

and that u, ε, and Ψare independent of z,

uα=uαrφ,εαβ=εαβrφ,Ψαβ=Ψαβrφ.E38

On the basis of these assumptions, we conclude (see Section A.2) that the physical components ΨαβγΨαβγhave the explicit form as follows:

Ψrrr=rΨrr,Ψrφφ=rΨφφ,Ψrrφ=rΨ,E39
Ψφrr=1rφΨrr2Ψ,E40
Ψφφφ=1rφΨφφ+2Ψ,E41
Ψφrφ=1rφΨ+ΨrrΨφφ,E42

whereas all other components of Ψvanish,

Ψαβz=Ψzαβ=0.E43

Similarly, we find (see Section 6.3) for the physical components ΔΨαβ=ΔΨαβ, that

ΔΨrr=rrΨrr+1r2φφΨrr+1rrΨrr4r2φΨ2r2Ψrr+2r2Ψφφ,E44
ΔΨφφ=rrΨφφ+1r2φφΨφφ+1rrΨφφ+4r2φΨ+2r2Ψrr2r2Ψφφ,E45
ΔΨ=rrΨ+1r2φφΨ+1rrΨ+2r2φΨrr2r2φΨφφ4r2Ψ,E46
ΔΨαz=0.E47

It is well known (see, e.g., Anderson [12], p. 114) that the nonvanishing physical components of εare given by the following expressions:

εrr=rur,εφφ=1rur+φuφ,ε=121rφur+ruφ1ruφ.E48

### 4.2 Cauchy stress: classical equilibrium equations

In view of the assumptions of the last section, we may derive the following results. We conclude from Eqs. (21)(23), that

Σαβ=Σαβrφ,ταβ=ταβrφ,σαβ=σαβrφ,E49

and that

Σαβ=ΣrrΣ0ΣΣφφ000Σzz,ταβ=τrrτ0ττφφ000τzz,E50
σαβ=σrrσ0σσφφ000σzz.E51

Since εzz=Ψzz=0, we deduce from the elasticity laws (21)(23) that

Σzz=νΣrr+Σφφ,τzz=ντrr+τφφ,σzz=νσrr+σφφ,E52

where νis given by Eq. (9). Thus, as in classical elasticity, once Σrrand Σφφhave been determined, Σzzis calculated by the first equation of (52).

Quite similar to the case of classical elasticity (see, e.g., Anderson [12], p. 114), the matrix of the components of Σin Eq. (50) and the classical equilibrium condition (24), expressed in physical components, lead to the following two equations:

rΣrr+1rφΣ+1rΣrrΣφφ=0,E53
rΣ+1rφΣφφ+2rΣ=0.E54

### 4.3 Classical compatibility condition

For the analytical solutions in Part II, we need the classical compatibility condition for the components of the strain tensor ε(see, e.g., Malvern [13], p. 669)

rrεφφ+1r2φφεrr2rε1rrεrr+2rrεφφ2r2φε=0.E55

The aim is now to rewrite this equation in terms of the physical components of Σand Ψby using Eq. (34). There are various equivalent representations for C1, depending on the chosen set of elasticity constants. We find it convenient here to express C1in terms of the elasticity constants μand ν. Thus, from Eq. (34), expressed in physical components,

εrr=c12μc2ΣrrνΣrr+Σφφ+c2c1c1Ψrr,E56
εφφ=c12μc2ΣφφνΣrr+Σφφ+c2c1c1Ψφφ,E57
ε=c12μc2Σ+c2c1c1Ψ.E58

By inserting these equations into Eq. (55), we get

rrc12μc2ΣφφνΣrr+Σφφ+c2c1c2Ψφφ2rc12μc2Σ+c2c1c2Ψ+1r2φφc12μc2ΣrrνΣrr+Σφφ+c2c1c2Ψrr1rrc12μc2ΣrrνΣrr+Σφφ+c2c1c2Ψrr+2rrc12μc2ΣφφνΣrr+Σφφ+c2c1c2Ψφφ2r2φc12μc2Σ+c2c1c2Ψ=0.E59

This is equivalent to a vanishing sum of two functions of Ψαβand Σαβ, respectively:

0=χ1Ψαβ+χ2Σαβ,E60

with

χ1Ψαβc2c1c2rrΨφφ2rΨ+1r2φφΨrr1rrΨrr+2rrΨφφ2r2φΨE61

and

χ2Σαβc12μc2rrΣφφνrrΣrr+Σφφ2rΣ+1r2φφΣrrνr2φφΣrr+Σφφ1rrΣrrνrrΣrr+Σφφ+2rrΣφφ2r2φΣ,E62

The right hand side of Eq. (62) can be simplified by invoking the equilibrium Eqs. (53) and (54). First recast Eq. (54) to solve for Σ,

Σ=r2rΣ12φΣφφ,E63

and then take the derivative with respect to φ,

φΣ=r2Σ12φφΣφφ.E64

On the other hand, from Eq. (53),

φΣ=rrΣrrΣrr+Σφφ,E65

and, after differentiation with respect to r,

Σ=rrrΣrr2rΣrr+rΣφφ.E66

By substituting the latter into Eq. (64),

φΣ=r22rrΣrr12φφΣφφ+rrΣrrr2rΣφφ.E67

Finally, by substituting Eqs. (66) and (67) into Eq. (62) and after some rearrangement of terms, we find that

χ2Σαβ= 1νc12μc2[rrΣrr+Σφφ+1r2φφΣrr+Σφφ+1rrΣrr+Σφφ].E68

### 4.4 Field equations for Ψ

By expressing C1in terms of μand νand using Eqs. (50), (37) and (44)(46), we can readily obtain from Eq. (35), expressed in physical components, the following three equations:

rrΨrr+1r2φφΨrr+1rrΨrr4r2φΨ2r2+1c2Ψrr+2r2Ψφφ+1ν2μc2Σrrν2μc2Σφφ=0,E69
rrΨφφ+1r2φφΨφφ+1rrΨφφ+4r2φΨ+2r2Ψrr2r2+1c2Ψφφ+1ν2μc2Σφφν2μc2Σrr=0,E70
rrΨ+1r2φφΨ+1rrΨ+2r2φΨrr2r2φΨφφ4r2+1c2Ψ+12μc2Σ=0.E71

### 4.5 Double stress

#### 4.5.1 Elasticity law for double stress

With respect to physical components, the elasticity law (24) becomes

μαβγμαβγ=c2c1ΨαρζCρζβγ=c2c12μΨαβγ+λΨαζζδβγ.E72

Keeping in mind that the physical components of Ψfor a plane strain state are given by Eqs. (39)(41), it is not difficult to derive the following results:

μrrr=c2c1λ+2μrΨrr+λrΨφφ,E73
μrφφ=c2c1λ+2μrΨφφ+λrΨrr,E74
μrzz=c2c1λrΨrr+Ψφφ=νμrrr+μrφφ,E75
μrrφ=c2c12μrΨ,E76
μφrr=c2c1r2μφΨrr2Ψ+λφΨrr+Ψφφ,E77
μφφφ=c2c1r2μφΨφφ+2Ψ+λφΨrr+Ψφφ,E78
μφzz=c2c1rλφΨrr+Ψφφ=νμφrr+μφφφ,E79
μφrφ=c2c1r2μφΨ+ΨrrΨφφ,E80
μrrz=μrφz=μφrz=μφφz=0,E81
μzαβ=0.E82

#### 4.5.2 Non-classical equilibrium conditions

The physical components of the non-classical equilibrium condition (26) are

div μαβ+σαβ=0.E83

With the aid of the physical components of μgiven by Eqs. (73)(81) and the physical components of σstated by Eq. (51), we can verify that the equilibrium conditions (83) furnish only four nontrivial equations:

div μrr+σrr=0,E84
div μφφ+σφφ=0,E85
div μ+σ=0,E86
div μzz+σzz=0,E87

or equivalently (cf. Section A.4)

rμrrr+1rφμφrr+1rμrrr2μφrφ+σrr=0,E88
rμrφφ+1rφμφφφ+1rμrφφ+2μφrφ+σφφ=0,E89
rμrrφ+1rφμφrφ+1rμrrφμφφφ+μφrr+σ=0,E90
rμrzz+1rφμφzz+1rμrzz+σzz=0.E91

### 4.6 Nonclassical compatibility conditions

Besides the classical compatibility condition for the strain εin Eq. (55), further compatibility conditions for the micro-strain Ψcan be established by considering the following identities:

ΨrrφrΨrr=0,E92
ΨφφφrΨφφ=0,E93
ΨφrΨ=0.E94

From these, we obtain useful relations by involving the physical components μαβγwith the aid of the elasticity law (24). To illustrate, we recall from Eqs. (39)(43) that

Ψrr=rφΨrr=rrΨφrr+2Ψ=Ψφrr+rrΨφrr+2ΨrrφE95

and that

φrΨrr=φrΨrr=φΨrrr.E96

By inserting these into Eq. (92), we obtain the following equation:

φΨrrrΨφrrrrΨφrr2Ψrrφ=0.E97

In a similar way, we conclude from Eqs. (93) and (94) that

φΨrφφΨφφφrrΨφφφ+2Ψrrφ=0,E98
φΨrrφΨφrφrrΨφrφ+ΨrrrΨrφφ=0.E99

In order to involve the components of μ, we invert Eq. (24) to obtain

Ψαβγ=1c2c1E1+νμαβγνμαζζδβγ,E100

where Eis given by Eq. (9). Explicitly, we get

Ψrrr=1c2c1E1ν2μrrrν1+νμrφφ,E101
Ψrφφ=1c2c1E1ν2μrφφν1+νμrrr,E102
Ψrrφ=1+νc2c1Eμrrφ,E103
Ψφrr=1c2c1E1ν2μφrrν1+νμφφφ,E104
Ψφφφ=1c2c1E1ν2μφφφν1+νμφrr,E105
Ψφrφ=1+νc2c1Eμφrφ,E106

where in addition use has been made of Eqs. (75) and (80). By inserting these components into Eqs. (97)(99), we can verify that

1ν2rrμφrr+ν1+νrrμφφφ+1ν2φμrrrν1+νφμrφφ1ν2μφrr+ν1+νμφφφ21+νμrrφ=0,E107
1ν2rrμφφφ+ν1+νrrμφrr+1ν2φμrφφν1+νφμrrr1ν2μφφφ+ν1+νμφrr+21+νμrrφ=0,E108
rrμφrφ+φμrrφμφrφ+μrrrμrφφ=0.E109

The last equation is independent of material parameters. In order to rewrite Eqs. (107) and (108) also in a form independent of material parameters, we add and subtract them from each other to obtain, respectively,

φμrφφ+φμrrrμφφφμφrrrrμφφφrrμφrr=0,E110
φμrφφφμrrrμφφφ+μφrrrrμφφφ+rrμφrr+4μrrφ=0.E111

### 4.7 Boundary conditions

As usually, near-tip field solutions rely upon boundary conditions, which are imposed only on the crack faces. Especially, we assume the classical traction P(see Eq. (27)) and the double force T(see Eq. (28)) to vanish on the crack faces. With regard to Figure 1 this implies that

Pαφ=±π=0,Tαβφ=±π=0.E112

Now, we have from Eq. (27), expressed in physical components, that Pα=nβΣβα, where on the crack faces nφ=±π=eφ. Therefore, and by virtue of Eq. (50), the nontrivial classical boundary conditions implied by Eq. (112) are as follows:

Σφ=±π=0,E113
Σφφφ=±π=0.E114

Similarly, we get from Eq. (28), expressed in physical components, that Tαβ=nγμγαβ, so that the nonclassical part of Eq. (112) implies

μφαβφ=±π=c2c1Ψφγζφ=±πCγζαβ=0,E115

where use has been made of the elasticity law (24). As the isotropic elasticity tensor Chas been assumed to be invertible, we infer from Eq. (115), that

0=Ψφαβφ=±π.E116

Keeping in mind Eqs. (39)(43), the only nontrivial conditions implied are as follows:

Ψφrrφ=±π=Ψφφφφ=±π=Ψφrφφ=±π=0,E117

or equivalently

φΨrr2Ψφ=±π=0,E118
φΨφφ+2Ψφ=±π=0,E119
φΨ+ΨrrΨφφφ=±π=0.E120

### 4.8 Symmetry conditions

Symmetry conditions are important to classify the near-tip field solutions into types according to Mode-I and Mode-II crack problems. Each type of loading condition is characterized by the following symmetry conditions.

#### 4.8.1 Mode-I

As in classical elasticity (see, e.g., Hellan [14], p. 10), we suppose for the macro-displacement the following symmetry conditions:

urrφ=urrφ,uφrφ=uφrφ,E121

i.e., uris an even function of φ, whereas uφis an odd function of φ. It follows from Eq. (48) that the physical components of the macro-strain εexhibit the following properties:

εrrrφ=εrrrφ,εφφrφ=εφφrφ,E122
εrφ=εrφ,E123

implying that εrrand εφφare even functions of φ, whereas εis an odd function of φ. Since Ψis also a strain tensor, we assume for its components, in analogy to Eqs. (122) and (123), that

Ψrrrφ=Ψrrrφ,Ψφφrφ=Ψφφrφ,E124
Ψrφ=Ψrφ.E125

Then, it can be verified, with the help of the elasticity law (21), expressed in physical components, that Eqs. (122)(125) engender the following conditions for the components of Σ:

Σrrrφ=Σrrrφ,Σφφrφ=Σφφrφ,E126
Σrφ=Σrφ.E127

Further, it can be seen from Eqs. (124) and (125), that

rΨrrrφ=rΨrrrφ,φΨrrrφ=φΨrrrφ,E128
rΨφφrφ=rΨφφrφ,φΨφφrφ=φΨφφrφ,E129
rΨrφ=rΨrφ,φΨrφ=φΨrφ,E130

and from the elasticity laws (73)(82), that

μrrrrφ=μrrrrφ,μφrrrφ=μφrrrφ,E131
μrφφrφ=μrφφrφ,μφφφrφ=μφφφrφ,E132
μrzzrφ=μrzzrφ,μφzzrφ=μφzzrφ,E133
μrrφrφ=μrrφrφ,μφrφrφ=μφrφrφ.E134

#### 4.8.2 Mode-II

We know from classical elasticity (see, e.g., Hellan [14], p. 10), that the radial component of the displacement vector is an odd function of φ, whereas the circumferential component is an even function of φ. We assume these symmetry properties to also apply for the macro-displacement here, i.e.,

urrφ=urrφ,uφrφ=uφrφ.E135

It follows for the macro-strain ε, that

εrrrφ=εrrrφ,εφφrφ=εφφrφ,E136
εrφ=εrφ,E137

which suggest to assume the following symmetries for Ψ:

Ψrrrφ=Ψrrrφ,Ψφφrφ=Ψφφrφ,E138
Ψrφ=Ψrφ.E139

It can be proved, in a similar fashion to Mode-I, that

Σrrrφ=Σrrrφ,Σφφrφ=Σφφrφ,E140
Σrφ=Σrφ,E141

and that

μrrrrφ=μrrrrφ,μφrrrφ=μφrrrφ,E142
μrφφrφ=μrφφrφ,μφφφrφ=μφφφrφ,E143
μrzzrφ=μrzzrφ,μφzzrφ=μφzzrφ,E144
μrrφrφ=μrrφrφ,μφrφrφ=μφrφrφ.E145

Before closing this section, we notice here, that the numerical simulations on the basis of the finite element method in Part IIIconfirm the assumed symmetry conditions.

## 5. Concluding remarks

If the implicit gradient elasticity model in Eq. (2), named the 3-PG-Model, is recognized as a particular case of micromorphic (micro-strain) elasticity, a free energy and associated response functions and boundary conditions can be assigned. Part Iadopts this conceptual point of view for the 3-PG-Model and provides the reduced form of the governing equations and boundary conditions for plane strain problems. This includes, among others, elasticity laws for classical and nonclassical stresses as well as classical and nonclassical equilibrium equations and compatibility conditions. It also supplies the required symmetry conditions for asymptotic solutions of Mode-I and Mode-II crack problems. A detailed discussion of such analytical solutions is given in Part II.

## Acknowledgments

The first and second authors thank the Deutsche Forschungsgemeinschaft (DFG) for partial support of this work under Grant TS 29/13-1.

This section provides the component representations with respect to cylindrical coordinates of some space derivatives of a second-order tensor Aand a third-order tensor A. It is easy to find component representations for Aand divAin textbooks, whereas it may be harder to find such representations for ΔAand divA. But one can calculate them with the help of the relations given below.

## A.1 Cylindrical coordinates

We denote by θithe cylindrical coordinate system with θ1=r,θ2=φand θ3=z. The covariant basis induced by θiis denoted by giwhere g1=cosφe1+sinφe2,g2=rsinφe1+rcosφe2and g3=e3. The contravariant basis is denoted by gi,gi=gijgj, where gijare the contravariant metric coefficients. The corresponding covariant metric coefficients are gij. All values of gijand gijare vanishing except for the values g11=g33=g11=g33=1,g22=r2and g22=1r2. Moreover, all values of the related Christoffel symbols Γijkalso vanish except for the values Γ221=rand Γ122=Γ212=1r. Physical components are referred to the orthonormal basis e<i>where e<1>er=g1,e<2>eφ=1rg2and e<3>ez=g3. According to Section 2, the physical components of a second-order tensor Aare denoted by Aαβand notations of the form A<11>Arr,A<12>A,apply. Similar notations hold also for any tensor, especially for the third-order tensor A. Finally, the nabla operator obeys the representation =θigi.

## A.2 The gradient of a symmetric second-order tensor

In the case of a second-order tensor A=Aijgigj, we have (cf. Section 2)

where Aijkis the covariant derivative of the components Ajk,

Aijk=Ajki=θiAjk+ΓimjAmk+ΓimkAjm.EA2

When Ais symmetric, A=As, we conclude from Eq. (A2), that

Aijk=Aijk.EA3

This symmetry also applies with respect to physical components,

Aαβγ=Aαβγ.EA4

It can be seen that Eq. (A2) furnishes the following physical components of A:

Arrr=rArr,Arφφ=rAφφ,Arzz=rAzz,EA5
Arrφ=rA,Arrz=rArz,Arφz=rAφz,EA6
Aφrr=1rφArr2Aφr,EA7
Aφφφ=1rφAφφ+2Aφr,EA8
Aφzz=1rφAzz,EA9
Aφrφ=1rφA+ArrAφφ,EA10
Aφφz=1rφAφzArz,EA11
Aφrz=1rφArzAφz,EA12
Azαβ=0.EA13

## A.3 The Laplacian of a symmetric second-order tensor

The Laplacian of a second-order tensor Ais given by (cf. Section 2)

This may be written as

ΔA=ΔAijgigj,EA15

where

ΔAij=Aijkmgkm,EA16

and Aijkmis the second covariant derivative of the components Aij,

Aijkm=Aijkm=θmAijk+ΓmliAljk+ΓmljAilkΓkmlAijl.EA17

We can calculate the physical components ΔA<ij>from Eqs. (A16) and (A17). For the case that Ais symmetric, A=As, we can derive, after lengthy algebraic manipulations, that

ΔArr= rrArr+1r2φφArr+zzArr+1rrArr4r2φA2r2Arr+2r2Aφφ,EA18
ΔAφφ= rrAφφ+1r2φφAφφ+zzAφφ+1rrAφφ+4r2φA+2r2Arr2r2Aφφ,EA19
ΔAzz=rrAzz+1r2φφAzz+zzAzz+1rrAzz,EA20
ΔA= rrA+1r2φφA+zzA+1rrA+2r2φArr2r2φAφφ4r2A,EA21
ΔArz=rrArz+1r2φφArz+zzArz+1rrArz2r2φAφz1r2Arz,EA22
ΔAφz=rrAφz+1r2φφAφz+zzAφz+1rrAφz+2r2φArz1r2Aφz.EA23

## A.4. The divergence of a third-order tensor

Let A=Aijkgigjgkbe a third-order tensor. Then (cf. Section 2)

divAA=giθiA=divAjkgjgk,EA24

where

divAjk=Aijki,EA25

and Aijkmis the covariant derivative of the components Aijk. If the symmetry condition AijkAijkholds, we can establish, after lengthy algebraic manipulations, the following results for the physical components of divA:

divArr=rArrr+1rφAφrr+zAzrr+1rArrr2Aφrφ,EA26
divAφφ=rArφφ+1rφAφφφ+zAzφφ+1rArφφ+2Aφrφ,EA27
divAzz=rArzz+1rφAφzz+zAzzz+1rArzz,EA28
divA=rArrφ+1rφAφrφ+zAzrφ+1rArrφAφφφ+Aφrr,EA29
divArz=rArrz+1rφAφrz+zAzrz+1rArrzAφφz,EA30
divAφz=rArφz+1rφAφφz+zAzφz+1rArφz+Aφrz.EA31

## How to cite and reference

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Carsten Broese, Jan Frischmann and Charalampos Tsakmakis (September 21st 2020). Mode-I and Mode-II Crack Tip Fields in Implicit Gradient Elasticity Based on Laplacians of Stress and Strain. Part I: Governing Equations [Online First], IntechOpen, DOI: 10.5772/intechopen.93506. Available from: