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Twin Boundary in hcp Crystals: Quantum and Thermal Behavior

Written By

Victor A. Lykah and Eugen S. Syrkin

Submitted: September 19th, 2018 Reviewed: May 17th, 2019 Published: June 22nd, 2019

DOI: 10.5772/intechopen.86909

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The 180° twin boundary (TB) (stacking fault) is investigated in the hexagonal close-packed (hcp) light materials. It is shown that atomic symmetry inside the twin boundary is lower than in hcp phase due to interatomic interaction between neighbors. In the case of quantum or thermal behavior, for the isosurfaces, an initial spherical form (in hcp phase) transforms into ellipsoid (in the boundary). We introduce the isosurface deformation parameter. The self-consistent description is developed to estimate the parameters of the thermodynamic potential, and the models of hard spheres and ellipsoids are used. It is shown that the quantum or thermal behavior of the boundary atoms causes the following effects: (i) the increase of degree of overlap of the atomic wave functions or trajectories within the twin boundaries, (ii) the increase of diffusion inside the twin boundaries, and (iii) the decrease of energy and broadening of the quantum boundary in comparison with the classical case.


  • solid helium
  • twin boundary
  • stacking fault
  • hard ellipsoids
  • quantum diffusionPACS numbers: 61.72.Mm
  • 61.72.Nn
  • 64.75.Gh
  • 66.30.Ma

1. Introduction

Helium crystals have unique quantum properties and are useful for the investigation of dynamic and kinetic behavior of atomic crystals [1]. In experiments, the structure phase transition between body-centered cubic (bcc) and hcp phase was found for both metals and solid 4He [2, 3]. The coherent phase boundary (PB) and twin boundary (TB) or stacking fault (SF) was investigated theoretically in the frame of one order parameter (OP) model [4, 5]. The two-OP theory of PB [6, 7] was developed on the basis of the Burgers mechanism. In work [5] we proposed the three-OP theory that combines Sanati [6, 7] and Kaschenko [8] treatments; so we take into account the changes of volume and pressure under the phase transition. The three-OP and one-OP descriptions of PB and TB are uniquely related. In different models of coherent bcc-hcp boundary, the local oscillations spectra of OP in 4He were investigated in [9].

In the experiment [10], a glass formation under deformation of solid helium was investigated. Usually the deformation of crystals generates the different defects [11], including stacking faults. In the nuclear magnetic resonance (NMR) experiments [12], the great role of the interface in increasing the quantum diffusion was found. In work [13] for single hcp crystal 4He, the stacking fault energy was measured.

The present work is devoted to the development of the self-consistent description of quantum behavior of 4He atoms in twin boundary proposed in work [14]. We apply this treatment to quantum and thermal description of twin boundary in some metals.


2. Model of the twin boundary

In the hcp phase of crystal 4He, we consider the twin boundary under transition from the close packing layers ABAB … (see Figure 1a,b) to the close packaging ACAC …. The twin boundary (TB) corresponds to stacking faults (SF). The atomic plane A creates different positions (potential wells) B and C for neighbor layers (see Figure 1a,b).

Figure 1.

(a, b) The close pack of the atomic layers (0001) ABAB… for hcp phase. Layer A is shown by solid lines, and layer B is shown by dotted lines. (a) The view perpendicular to the layers. (b) The view along the layers. Points B and C are atomic equilibrium positions in corresponding layer. (c, d) The change in the close packing of the atomic ellipsoids inside TB under quantum effects is accounted.

The twin boundary was researched in works [4, 5] where the triple-well thermodynamic potential was used. Far from the bcc-hcp transition, the double-well free energy can be applied:


where the integration is over the volume v, square brackets contain the volume energy density, zis a coordinate in the direction of heterogeneity, αis a dispersion parameter responsible for the boundary width, and phenomenological parameters k4,k2are positive. In hexagonal lattice, ξis the order parameter which means the relative displacement of the atomic layers between positions B and C (see Figure 1a,b). For the homogeneous part of the free energy Eq. (1), the maximum and minima positions are


where ξ0is the minimum position as displacement between the maximum and minimum positions (Band Cin Figure 1a,b). The difference between the maximum and minimum energies gives the height hof the potential barrier per unit volume:


For further analysis it is convenient to write the free energy Eq. (1) in terms of ξ0and h:


The free energy Eq. (4) gives rise to such one-dimensional inhomogeneity as twin boundary [9, 15] which has shape


where the boundary center is chosen at z=0and lTis the characteristic width of the boundary. The shear dependence on coordinate Eq. (5) can be substituted into relation Eq. (4). The surface energy density of the twin boundary is obtained by further integration:


It is expressed through parameters αk2k4of the microscopic double-well potential or macroscopic parameters lTh. The parameters of the thermodynamic potential Eq. (1) can be transformed into the microscopic ones:


Here h1, k21, and k41 are the barrier height Eq. (3), parameters k2 and k4 Eq. (1) normalized per unit cell. These equalities are obtained by multiplying hand k2or k4to the unit cell volume v1. The characteristic width Eq. (6) lT1.5nmwas obtained by molecular dynamic method in [16].


3. Atomic potential in continual description

In hcp lattice, one can find the symmetry axes (along 0z) of third and sixth orders. In the close-packed layers xy, hcp demonstrates isotropic properties of macroscopic tensors [11, 17]. The isotropic macroscopic tensors exist at appropriate relations c/a=8/3of unit cell sizes [1, 11]. Inside the perfect hcp phase, an atom is in high symmetric (isotropic) potential:


where kisis isotropic rigidity. The harmonic approximation Eq. (9) is satisfied better for heavier inert atoms or light metals; however, the helium crystal has pronouncedly anharmonic atomic potential [18]. Nevertheless in helium crystals, the harmonic approximation is successfully applied [19, 20].

The isotropic rigidity kiscan be divided into two contributions: kis=kp+kpn, where kpis rigidity in the plane and kpnis rigidity from the interaction with the neighbor planes.

Inside the twin boundary, the neighbor layers are shifted from the symmetric positions, and it causes an anisotropic atomic potential. The previous spherical potential is broken. Then inside the twin boundary, the initial isotropic atomic potential transforms into


where the isotropic potential Eq. (9) splits into two terms. The first term Uan1xis an anisotropic and nonlinear part of the potential in the shift direction Ox. The second term Uisyzis the rest of the isotropic part which is perpendicular to the shift direction. Further, the potential Uan1xis divided too into Upx, the isotropic part, and Upnxξ, the anisotropic one from the neighbor atomic planes. The last turn depends on the layer shift ξand the small deviation x. Therefore, only term Upnxξchanges inside TB which is shown in Figure 2. The analysis (see [14]) of the term Upnxξallows to write the anisotropic atomic potential Eq. (10) in the following simple form:

Figure 2.

Smooth changed parts of the potential in dependence on the coordinatesξandxaccording toEqs. (10)and(11):Upn0ξis a lower double-well curve andUan1xξis a set of parabolas.


where kbξis rigidity coefficient inside TB, U0ξis a varied bottom level, and cξxis the linear part. In the limit points ξ=±ξ0, Eq. (11) transforms into isotropic hcp phase Eq. (9) with kpnξ0=+2k21. Inside TB ξ=0, the rigidity takes value kpn0=k21. Thus, the rigidity coefficients in phase kisand in the middle of TB kb0are represented by the rigidity coefficients inside the plane kpwith two adjacent k21planes:


Inside the boundary the potential is considerably softer in direction Oxbecause of kbξ<kis(see Figure 2). The difference in these rigidity coefficients is too high kiskb0=3k21. For further analysis, we need especially the quadric form in Eq. (11).

The ratio of the rigidity coefficients in the relation Eq. (10) can be related to the ratio of the elastic modules which are shown in Table 1. The macroscopic tensor components C11C33describe the longitudinal deformation along the axes 0xand 0z, respectively. In solid 4He, the ratio of the elastic modulus C33/C11=1.37gives anisotropy of the rigidity coefficients kelz/kisin the basal plane and axis 0z. Uniaxial compression-tension in the basal plane of 0xycorresponds to the elastic modulus of C11 and atomic rigidity coefficient kis. The shuffle of the basal planes in an arbitrary direction corresponds to elastic modulus C44and atomic rigidity coefficients 2k21. Therefore, we have the following inequality:

ElementC11, GPaC33, GPaC13, GPaC44, GPa
4He [21] a4:05·10−25:54·10−21:05·10−21:24·10−2
7Li [22] b14.210.7
9Be [23] b2923496163
24Mg [23] b59.361.521.416.4

Table 1.

The experimental values of the elastic moduli of some hcp materials in the notation of Voigt Cikfollowing [11].

The elastic moduli of hcp 4He are found at T1Kand molar volume 20.97106m3/mo1[21].

At room temperature.


4. The atomic potential and hard sphere model in hcp phase

The geometry of the hcp lattice is shown in Figure 1a. In the hard sphere model for the hcp plane A (see Figure 1a,b), the coordinates of atomic centers are


where R0 is the atomic radius, xis a coordinate along the shift direction of the atomic plane B, zis a coordinate along the direction perpendicular to the atomic plane, and yis a coordinate along the atomic plane perpendicular to the shift direction. (0,0,0) is the touch point of the spheres in plane A. Then the sphere centers of the shifting atomic plane B can move over the following four spherical surfaces:


The equilibrium points for the atom of the shifting neighbor atomic plane B can be found from the geometry of the system (Eq. (16) at y=0):


Signs – and + in xRedescribe positions B and C in plane B, respectively. From the first Eq. (16), the saddle point coordinates for an atom of plane B are


For the hard sphere model, the microscopic parameters ξ0,h1are


where h1Ris the potential barrier between B to C position (see Figure 1). Coefficient g1evaluates the quasielastic energy. In the middle of TB, the neighbor number is 4, which is less than 6 once inside the phase. This is a microscopic reason for the quasielastic energy behavior.

For the hard sphere model, the substitution of relations (19) into Eqs. (3) and (8) gives the parameters of the microscopic interatomic potential:


For comparison, Eq. (11) allows us to find the rigidity coefficients in the phase kisand in the middle of the boundary kb0.


5. Quantum atomic spheres and ellipsoids in hcp phase and in the twin boundary

Inside the perfect hcp phase, a 4He atom is in highly symmetric potential of neighbor atoms. In isotropic harmonic approximation [19, 20], the atomic potential can be presented as [24]


where m,rand λare mass, radius vector of 4He atom and parameter of the quantum oscillator. The potential Eq. (12) gives mω2=kis;λ2=kism/2.

The Schrodinger equation splits into three equivalent independent equations with the constant k2=kX2+ky2+kz2=2mW/2where kiare wave numbers. The ground state solution [24] has total zero-point energy W0is=32ω. In isotropic harmonic approximation, a distribution of probability density ρ=ψxyz2of helium atom has spherical symmetry. Hence, the equation of probability isosurface (sphere of radius R) is


The probability density at a distance of R0 that equals to the radius of the atom in the hcp phase (half the distance between the centers of neighboring atoms in the crystal) is


Here we have introduced the dimensionless parameter κ0that is important for further consideration. This parameter is proportional to the atomic radius κ0R0and depends on the isotropic rigidity of the atomic lattice κ0λ1/2kis1/4. In respect to a huge change in the volume of solid helium [1], the parameter κ0can vary widely.

An anisotropic harmonic potential can be written as [24]


The parameters λiare related to the rigidity coefficients:


In the hcp phase, an anisotropic harmonic approximation is more adequate. Then the rigidity coefficients satisfy inequality kxel=kyel=kis<kzel. If we use isotropic harmonic approximation in the hcp phase, then inside of the twin boundary, an atom 4He is in a uniaxial potential of neighboring atoms of Eq. (13): kxel=kbkyel=kzel=kis.

The equation splits also into three independent equations with known solutions [24]. Inside TB for the ground state, the distribution of the probability density of the helium atom loses its spherical symmetry. The probability isosurface is ellipsoid with semiaxes abc:


Parameter Nρdescribes the probability density. If the probability density equals ρ0at the atomic radius R0 in the hcp phase Eq. (23), then Nρtakes the following value:


Thus, the relations Eqs. (26) and (27) describe the probability density isosurfaces to find an atom in the anisotropic case. On appropriate limit λi=λ, these relations describe the isotropic case.


6. Classic atomic thermal spheres and ellipsoids in hcp phase and the twin boundary

Inside the perfect hcp phase, an atom is positioned in highly symmetric potential of neighbor atoms (see Eq. (9)) and quantum analogue Eq. (21). For any direction, the average thermal energy of an atom is kBT/2where kBand Tare the Boltzmann constant and temperature.

In isotropic harmonic approximation Eq. (9), the average thermal energy of an atom corresponds to the average potential isosurface (sphere of radius R):


The general anisotropic potential has form Eq. (10). In anisotropic harmonic case, the potential can be written with corresponding rigidity coefficients as (compare with Eq. (24))


Then inside of the twin boundary, an atom is in the uniaxial potential of neighboring atoms Eq. (13): kxel=kbkyel=kzel=kis.

The motion equation splits also into three independent equivalent equations. The equation of the potential isosurface is ellipsoid with semiaxes abc(compare with Eq. (26)):


Thus, the relation Eq. (30) describes the atomic potential isosurfaces in the anisotropic case, i.e., inside TB. In the limit case ki=kis, it corresponds to the isotropic case, i.e., hcp phase Eq. (28). The thermal potential isosurfaces (ellipsoids) have to be in order less than the quantum atomic spheres and ellipsoids normalized at R0. We emphasize that in this section the average thermal motion of atoms was considered.


7. The self-consistent description of the twin boundary

The classic descriptionof TB uses two coefficients of the thermodynamic potential Eq. (1):


They can be corresponded to the hard sphere model (see Eqs. (15)(20)).

The quantum and thermal descriptionof TB is self-consistent, i.e., the parameters Eq. (31) are varied as a function of some parameter qthat, in its turn, is a function of these parameters:


Let us introduce the isosurface deformation parameterqas a geometric factor which describes the deformation of the atomic sphere Eqs. (22) and (28) into the one-axis ellipsoid Eqs. (26) and (30):


where εis the eccentricity of the ellipse. Earlier in the paper [14], we introduced the quantum deformation parameter qq. Here we generalize the parameter qqto the cases of either quantum or thermal motion of an atom and introduce the isosurface deformation parameter q.

Now we present the self-consistent scheme of description for the twin boundary.

  1. (0) Zero approximation. An atom is a hard classic sphere Eq. (32) or quantum isotropic oscillator:


  1. (1) The first approximation. An atom is considered as a quantum anisotropic uniaxis oscillator. The potential Eq. (10) has been obtained in zero approximation. In the general case, the ellipsoid parameters and the isosurface deformation parameter are described by Eqs. (26), (27), and (33), respectively. The long ellipsoids axis is oriented along the shift direction 0x:


  1. The further variations of parametersEq. (31) can be obtained in the hard ellipsoid model. The hard ellipsoids have the isosurfaces with the same probability density ρ0as the hard spheres in the hcp phase, and the isosurface deformation parameter can be obtained. For a vacancy, the nearest neighbors form similar ellipsoids [25].

  2. (2) The second approximation. An atom is considered as an anisotropic three-axis oscillator (the isosurface is three-axis ellipsoid). The first approximation gives the rigidity coefficients of the potential. Different ellipses are formed in the planes aband ac, and their eccentricities equal


  1. Now all three axes of the atomic ellipsoid are different. The softest potential and the longest axis a2 are still oriented along the shift direction. The hard ellipsoid model Eq. (35) is used to obtain a new local atomic potential and a new ellipsoid shape.

  2. (i) The third and further ith steps qualitatively replicate the previous steps in the same way. The second and further steps are more cumbersome and complicated.


8. Atom as anisotropic harmonic oscillator in the boundary, one axis

In continual description inside the boundary, we have found a change of the atomic potential Eq. (10) with the corresponding rigidity constants. Therefore, constants λiin Eq. (25) take the following forms:


Using Eqs. (26) and (27), the atomic isosurface can be described by ellipsoid with semiaxes:


For fixed λy,λz=λand reduced stiffness coefficient λXalong axis 0x, the semiaxes of the ellipsoid change as follows: a1>R0;b1=C1<R0. Then the isosurface deformation parameter q1 Eq. (35) takes the following dependence on the order parameter ξand coordinate


We obtain the same result for the thermal excitations; however, instead of relation Eq. (37), we use the rigidity constants Eq. (30):


In Table 2, evaluations of different parameters are shown according to Table 1 and relation Eqs. (14), (39), (42), and (43); the sources are shown in round brackets on top of columns.

ElementC44C11, (Table 1, (14))3k21kis, Eq. (14)qmax, Eq. (39)κ02, Eq. (42)Λ, Eq. (43)

Table 2.

Evaluation of the elastic moduli relations, rigidity relations, the isosurface deformation parameter in the middle point of TB qmax, and the de Boer parameter Λof some hcp materials.

Evaluation of the de Boer parameter Λ=0.45for 4He at ∼1 K [2].

At room temperature.

Evaluation of the de Boer parameter at 1K(present work).

For all materials the parameters κ02and Λare evaluated with the same R0.

In He and Mg (see Table 2), the transverse components of the elastic module C44 are much smaller than the longitudinal ones C11. Accordingly in these materials, the isosurface deformation parameters in the middle point of TB qmaxtake relatively small value.

In Li and Be (see Table 2), the transverse and longitudinal components of the elastic moduli are closer. Hence, in these materials, the parameters qmaxare considerably greater. Moreover in Li, the parameter qmaxcan reach 1 or even take complex (imaginary root) values. This indicates a possible instability of Li crystal lattice (see further consideration). This, seemingly unexpected, result is quite understandable if considerably gentle upper parabolas (stronger interaction between the crystal planes in comparison with in-plane interaction) are taken into account which are shown in Figure 2.

In the quantum case, we can evaluate the minimal increase of the exchange integral due to the increase of overlapping wave functions caused by the elliptic deformations [14]:


Increasing overlapping volumes ΔVwith high probability can be evaluated by segments of the crossing ellipsoids. Amplitude ΔI0depends on two parameters κ0and k21/kisonly.

In the basal hcp plane, the exchange integral is varied depending on the quantum deformation parameter q; the wave function tails are the most sensitive, especially in the overlapping region. Evaluations Eq. (41) take into account only space changing but not the amplitude one. The amplitude changing can achieve several orders because of exponential dependence. The exchange integral Iuniquely defines the diffusion coefficient [26]. In the interphase boundaries in solid helium, NMR experiment [12] shows the quantum diffusion increasing. The interphase and twin boundaries are similar [5]. So for the quantum diffusion case in TB, the predicted and the experimentally observed arising values are closely related. Experiments show thermal diffusion arising at boundaries [11]; the found thermal ellipsoids’ deformation qualitatively explains these facts.

Now we can point out conditions when exchange integral Eq. (41) increases. We need minimal κ02Eq. (42) in exponent Eq. (41). The parameter κ0or λcan be defined by Eqs. (23) and (37) and analyzed in dependence on different factors. In [14] using atomic mass maand evaluation of atomic radius R0, the parameter κ02value was estimated:


where elastic module E=C11is related to the rigidity coefficient kisπR0E/2. In solid 4He, the atomic radius R0is the soft parameter, especially under low pressure. So, a high value of exchange integral can be achieved. Compressibility is small in metals, first of all, in light ones (lithium, beryllium, magnesium). Minimal rigidity kisgives rise in the exchange integral too. The van der Waals interaction in 4He is 3–4 orders of magnitude less than in metal (see Table 1).

Another way to estimate κ02is to compare it with de Boer parameter Λ, the fundamental characteristic of quantum crystal. The de Boer parameter gives the probability density to find an atom in the site of a neighboring atom (at distance al=2R0) [26]:


The de Boer parameter Λ=0.45for 4He [26] gives evaluation κ020.59. Pressure growing leads to more difficult tunneling of atoms and different κ02evaluations in Eqs. (42) and (43). Using the data in Table 1, for solid 4He we obtain R0[14], κ023.77, and Λ0.07(see Table 2).

We can make the following conclusion. The softening of the effective atomic potential is anisotropic inside the twin boundary which increases the exchange integral and tunneling probability in the selected shear direction. As a result the quantum diffusion along the boundary plane increases.


9. The self-consistent correspondence of the potential and the uniaxial hard ellipsoid model

Inside the twin boundary, the arising anisotropic atomic potential transforms an atomic probability isosurface from sphere to ellipsoid. Let us introduce the hard ellipsoid model as analogue of the hard sphere model. Then coefficients’ local values for the potential can be found inside TB. We suppose that the twin boundary does not change symmetry and positions of the atomic centers inside a shifting plane. So, the atomic plane A keeps the atomic centers’ coordinates Eq. (15) under shifting (see Figure 1c,d). In the shifting neighbor atomic plane B, the atomic isosurface equation is defined by Eq. (22). Then for the shifting atomic plane B, the atomic (ellipsoids) center moves over the great ellipsoidal surfaces:


where the equilibrium and saddle points for an atom are located. Only four ellipsoids with centers 0±R00and ±R03,0,0are described. Axis 0xis directed along the shift (see Figure 1c,d).

Relations Eq. (26), (27), and (35) define the ellipsoid’s semiaxes as function of R0,q:


Accounting these relations and condition y=0(see Figure 1), we obtain solution for the equation system Eq. (44) and the equilibrium point coordinates for the atom of the plane B. So, in the hard ellipsoid model, we find the microscopic parameters Eqs. (2) and (3) of the atomic potential:


where h1Ris defined in Eq. (19). These results are valid in the range 0q2/3. At q12/3we have ξ01,h110and semiaxis relation a1/c1=1/3. At q=2/3the hard ellipsoid model needs transition in another state (see [14]). Therefore, inside TB, the change of the atomic wave function leads to the following change of the interaction potential: the equilibrium displacement and the potential barrier height decrease (see Figure 3). However, the potential barrier height decreases much faster. The resulting evolution of the potential Eq. (46) is shown in Figure 4. Then from Eqs. (3) and (46), the coefficients of the potential are

Figure 3.

Comparison of the hard ellipsoids model and the atomic microscopic potential. The red double-well curve shows the potential as a function ofξ01andh11. Small solid red ellipsoids show atomic isosurfaces atκ0. Big dot black ellipsoids show the cross sections of the surfacesEq. (44)aty=0and quantum parameter values (a) q = 0, (b) q = 0.2, (c) q = 0.4, and (d) q = 0.6.

Figure 4.

The cross sections of the potential density according toEqs. (46),(47), and(39). The quantum boundary has lower potential peak and shorter distance between shallower wellsξ01as q grows (0, 0.2, 0.4, 0.6). The barrier in the middle of wall (TB) decreases.


Thus, the coefficients of the potential (1) for the shift in the direction 0xreduce k21>k211qand k41>k411q. It means softening of the potential in the direction of the plane shuffle. The correspondence between the hard ellipsoid model and the atomic microscopic potential Eqs. (4), (8), and (46) is shown in Figure 3. Elliptical deformation of the probability isosurface leads to the transformation of the potential energy of the atom in Eq. (10):


All terms are changed in the potential Eq. (48) in comparison with Eq. (10). Isotropy is broken in atomic planes A or B-C due to superposition of the ellipsoids in the shear direction.

For the classical and quantum cases, the free energy density relation Eq. (4) was analyzed analytically in [14]. It was shown that the classical and quantum boundaries have different properties. In particular, from Figure 5, it is qualitatively clear why the classical and quantum boundaries have different potential barrier and energy density. In TB both the width and the height of the barrier decrease to zero, according to Eqs. (46) and (47) (see Figure 4). In Figure 3, they are shown as higher smooth curves. Simultaneously the space width of the boundary lT=1/ξ02α/k4grows by Eq. (6). The dependence lTqcauses further widening of region with qqmaxand a minimal barrier height.

Figure 5.

The smooth double-well potential according toEqs. (10)and(11). Instead of a set of parabolas inFigure 2, we see only ones at the bottom and the peaks of the potential and their quantum levels. The relationship between the barriers for the atomic displacement in the classicalhcand quantumhqboundaries ishc>hq.

To estimate the energy of the twin boundary (stacking fault) from Eq. (7), we must know the following parameters: α,k2,k4or lT,h.

The characteristic width (half width) of TB Eq. (6) lT1.5nm was obtained by molecular dynamic method in [16]. We estimate the dispersion parameter αby comparing the differential equations for the transverse sound and shuffling waves:


where ρ=ρ/2is the effective density of the oscillating shuffled subsystem, ρis the density of helium-4, ξis the shuffling order parameter, uis macroscopic displacement, and s=C44/p255m/sis the transverse sound velocity in the shuffle direction (Ozaxis). The velocities of transverse sound and shuffling wave have close values. So the dispersion parameter is αC44/2=6.2106J/m3where value of module C44 is given in Table 1.

According to relation Eq. (5), it is possible to estimate the parameter of the thermodynamic potential k2=2α/lT28.271024J/m5. As follows from Eq. (2) to evaluate the parameter k4 of the potential, it is necessary to know the maximum displacement of the atom Eq. (17) ξ0=R0/31.171010m. Here atomic radius is related to atomic volume: Vm/NA4/3πR03. Then k4=2α/ξ0lT2=6.041044J/m7. So, for the classical model of the twin boundary (stacking fault), it is possible to estimate bulk density of the barrier height hand the surface energy density WTaccording to Eqs. (3) and (7):


The surface energy density calculated here for the classical model can be compared with the value WSFex=0.07±0.02mJ/m2found in the optical experiments at 0.2 K [13].

Above, we have predicted the local reduction of the barrier height hand a local increase in the width lTof the boundary in the quantum description of the twin boundary (stacking fault). In general for the defect, the surface energy density value WTlTefhTefin Eq. (50) can be close to the classical case. In different experiments and theoretical estimates, a wide variation of the values may be caused by variations of temperatures and pressures.

We have discussed the change of zero vibrations of atoms in the twin boundary (stacking fault) and the related effects. For 3He we can expect the same order of magnitude for all parameters of the twin boundary (stacking fault). The qualitative difference between the pure hcp crystals of isotopes 4He and 3He, apparently, cannot be obtained in the proposed model.

The difference between quantum statistics of the isotopes should address deeper and more delicate quantum properties of the defects. We note briefly below only the most striking manifestation of different statistics and problems arising in this regard.


10. Discussion and conclusion

The quantum self-consistent treatment to twin boundary (stacking faults), proposed in [14] for solid 4He, is developed here for metals and their quantum and thermal description. The relation between discrete models of hard spheres and continuum interatomic potential is used as a sample for a similar relationship in the case of the hard ellipsoid models. As we move deeper into the defect, the transition from one model to another is accomplished.

In the hcp phase, the potential of an atom, created by its neighbors, has spherical symmetry (initial approximation). In the hcp phase, an atom is an isotropic quantum oscillator. In the twin boundary, an atom is an anisotropic quantum oscillator. It is shown that in the twin boundary, the potential of the atom is softer in the direction of shuffle of the atomic planes.

The quantum parameter qqand its generalization and the isosurface deformation parameter qare introduced. These parameters have simple and visual meaning: qequals to the square of the eccentricity of the cross section of the probability density ellipsoid (or the thermal ellipsoid). We have shown that parameter qis associated with de Boer parameter, the fundamental characteristic of quantum crystal, and anisotropy in the boundary. Evaluations for different materials show that the isosurface deformation parameter qcan achieve values 0.2÷1(see Table 2). Meanwhile at q=2/3the structure instability takes place in the system of the atomic ellipsoids. From this point of view, the properties of TB in lithium are especially interesting because the parameter achieves high value q1.

The overlap of the atomic wave functions and the exchange integral value can be described in terms of the quantum parameter q. Inside the twin boundary, the quantum diffusion increases which was observed in the phase boundary (see experiment [12]). The estimation Eq. (50) of the defect energy is in good agreement with experiment [13]. We have shown that the quantum deformation of atoms leads to the space broadening of the twin boundary and to its energy decreasing.

In conclusion we note that local oscillations spectra of the order parameter in different models of coherent bcc-hcp boundary in 4He were investigated in [9]. For small values of the perturbations, dynamical differential equations (reduced to Schrodinger equations) were obtained and solved. The characteristic frequencies (energy levels) and shape were found and estimated (see Figure 6). For the ground state in TB, the local vibration shape can be written as

Figure 6.

Local modes of the order parameter at TB [9]. Dash dot line shows the local potential which has local energy levels 0, 1, and 2 (dash). Solid lines show corresponding local oscillations’ shape dependence on normalized coordinatez.


where A0is an amplitude. For the local vibration ground state (51) and for the isosurface deformation parameter qEq. (39), both shapes coincide qualitatively. In the limit q<<1, both coincide completely. The local vibration of the order parameter describes a correlated motion of the atomic layers in twin boundary. Meanwhile, the quantum and thermal treatments give probabilistic descriptions of the atomic motion. The results (the found smooth arising of the atomic motion amplitude in TB) give evidence that different probabilistic (quantum and thermal) and dynamic methods lead to qualitatively identical features of the atomic basic state inside TB.


This research is supported by the FFI National Academy of Sciences of Ukraine, grant 4/18-H, Ministry of Science and Education of Ukraine under the Projects M05486 (0118U002048).


  1. 1. Maradudin AA. In: Freiman YA, Manzhelii VG, editors. Physics of Cryocrystals. AIP Press: New York, Woodbury; 1996. p. 691. DOI: 10.1007/1-56396-537-2
  2. 2. Maekawa M, Okumura Y, Okuda Y. Nucleation of crystals at the bcc-hcp transition line in solid 4He. Physical Review B. 2002;65:144525. DOI: 10.1103/PhysRevB.65.144525
  3. 3. Birchenko AP, Vekhov EO, Mikhin NP, Polev AV, Rudavskii EY. Kinetics of the bc-chcp transition in 4He off the melting curve. Low Temperature Physics. 2006;32:1118-1112. DOI: 10.1063/1.2400684
  4. 4. Lykah VA, Syrkin ES. Twin boundaries as nuclei of a new phase in body-centered cubic-hexagonal close-packed phase transitions in solid helium. Physics of the Solid State. 2010;52:384-391. DOI: 10. 1134/S1063783410020265
  5. 5. Lykah VA, Syrkin ES. Theory of the phase and twin boundaries in solid helium and reversibility of the bcc-hcp phase transition. Journal of Low Temperature Physics. 2010;160:179-194. DOI: 10.1007/sl0909-0l0-0l9l-6
  6. 6. Sanati M, Saxena A, Lookman T, Alberts RC. Landau free energy for a bcc-hcp reconstructive phase transformation. Physical Review B. 2001;63:224114. DOI: 10.1103/PhysRevB.63.224114
  7. 7. Sanati M, Saxena A, Lookman T. Domain wall modeling of bcc to hcp reconstructive phase transformation in early transition metals. Physical Review B. 2001;64:092101. DOI: 10.1103/PhysRevB.64.092101
  8. 8. Kaschenko MP, Chaschina VG. Crystal dynamics of the BCC-HCP martensitic transformation: I. controlling wave process. The Physics of Metals and Metallography. 2008;105:537-543. DOI: 10. 1134/S0031918X08060021
  9. 9. Lykah VA, Syrkin ES. Local oscillations in different models of coherent bcc-hcp boundary in 4He and metals. Physica Status Solidi B. 2011;248:1392-1398. DOI: 10. 1002/pssb.201046304
  10. 10. Lisunov AA, Maidanov VA, Rubanskyi VY, Rubets SP, Rudavskii EY, Rybalko AS, et al. Features of the temperature dependence of pressure of solid helium at low temperatures. Low Temperature Physics. 2012;38:459-465. DOI: 10.1063/1.4723660
  11. 11. Kittel C. Introduction to Solid State Physics. 8th ed. New York: Wiley; 2004. p. 704
  12. 12. Vekhov EO, Birchenko AP, Mikhin NP, Rudavskii EY. Fast diffusion process in quenched hcp dilute solid 3He-4He mixture. Journal of Low Temperature Physics. 2010;158:496-501. DOI: 10.1007/sl0909-009-0022-9
  13. 13. Junes HJ, Alles H, Manninen MS, Parshin AY, Todoshchenko IA. Stacking fault energy in 4He crystals. Journal of Low Temperature Physics. 2008;153:244-249. DOI: 10.1007/sl0909-008-9828-0
  14. 14. Lykah VA, Syrkin ES. Quantum behavior of the twin boundary and the stacking fault in hcp helium crystals. Journal of Low Temperature Physics. 2015;181:10-29. DOI: 10.1007/sl0909-015-1328-4
  15. 15. Lines ME, Glass AM. Principles and Application of Ferroelectrics and Related Materials. 2nd ed. Oxford: Clarendon; 2001. p. 683. DOI: 10.1093/acprof:oso/9780198507789.001.0001
  16. 16. Ceperley D. Supersolid: Crystal or plastic? Nature Physics. 2006;2:659-660. DOI: 10. 1038/nphys424
  17. 17. Landau LD, Lifshitz EM. Theory of Elasticity. 3rd ed. Vol. 196p. New York: Pergamon; 1986. DOI: 10.1007/978-0-7506-2633-0
  18. 18. Guyer RA. The theory of quantum crystals. In: Seitz F, Tumbull D, Ehrenreich H, editors. Solid State Physics. Vol. 23. New York: Academic Press; 1969. pp. 413-499. DOI: 10.1016/S0081–1947(08)60618–9
  19. 19. Ebner C, Sung CC. Correlation effects in quantum crystals. Physical Review A. 1971;4:269-281. DOI: 10.1103/PhysRevA.4.269
  20. 20. Gov N, Polturak E. Local modes, phonons, and mass transport in solid 4He. Physical Review B. 1999;60:1019-1027. DOI: 10.1103/PhysRevB.60.1019
  21. 21. Greywall DS. Elastic constants of hcp 4He. Physical Review B. 1977;16:5127-5128. DOI: 10. 1103/PhysRevB. 16.5127
  22. 22. Day JP, Ruoff AL. The variation of the elastic constants of lithium with temperature and pressure. Physica Status Solidi. 1974;25:205-213. DOI: 10. 1002/pssa.2210250118
  23. 23. Tromans D. Elastic anisotropy of hcp metal crystals and polycrystals. International Journal of Research and Reviews in Applied Sciences. 2011;6:462-483. Available from: 6Issue4/IJRRAS_6_4_14.pdf
  24. 24. Flugge S. Practical Quantum Mechanics. 2nd ed. Berlin: Springer; 1999. p. 635. DOI: 10.1007/978-3-642-61995-3
  25. 25. Guyer RA, Richardson RC, Zane LI. Excitations in quantum crystals (A survey of NMR experiments in solid helium). Reviews of Modern Physics. 1971;43:532-600. DOI: 10.1103/RevModPhys.43.532
  26. 26. Andreev AF. Diffusion in quantum crystals. Soviet Physics Uspekhi. 1976;19:137-148. DOI: 10.1070/PU1976v019n02ABEH005133

Written By

Victor A. Lykah and Eugen S. Syrkin

Submitted: September 19th, 2018 Reviewed: May 17th, 2019 Published: June 22nd, 2019