Polarizability and Impurity Screening for Phosphorene

Po Hsin Shih,Thi Nga Do, Godfrey Gumbs and Dipendra Dahal

#### Abstract

Using a tight-binding Hamiltonian for phosphorene, we have calculated the real part of the polarizability and the corresponding dielectric function, Re[ϵð Þ q;ω ], at absolute zero temperature (T = 0 K) with free carrier density 10<sup>13</sup>=cm2. We present results showing Re[ϵð Þ q;ω ] in different directions of the transferred momentum q. When q is larger than a particular value which is twice the Fermi momentum kF, Re [ϵð Þ q;ω ] becomes strongly dependent on the direction of q. We also discuss the case at room temperature (T = 300 K). These results which are similar to those previously reported by other authors are then employed to determine the static shielding of an impurity in the vicinity of phosphorene.

Keywords: phosphorene, polarizability, impurity screening

#### 1. Introduction

Emerging phenomena in physics and quantum information technology have relied extensively on the collective properties of low-dimensional materials such as two-dimensional (2D) and few-layer structures with nanoscale thickness. There, the Coulomb and/or atomic interactions play a crucial role in these complexes which include doped as well as undoped graphene [1–3], silicene [4, 5], phosphorene [6, 7], germanene [8, 9], antimonene [10, 11], tinene [12], bismuthene [13–18] and most recently the 2D pseudospin-1 α � T<sup>3</sup> lattice [19]. Of these which have been successfully synthesized by various experimental techniques and which have been extensively investigated by various experimental techniques, few-layer black phosphorus (phosphorene) or BP has been produced by using mechanical cleavage [6, 20], liquid exfoliation [7, 21, 22], and mineralizer-assisted short-way transport reaction [23–25].

Unlike graphene, phosphorus inherently has an appreciable band gap. The observed photoluminescence peak of single-layer phosphorus in the visible optical range shows that its band gap is larger than that for bulk. Furthermore, BP has a middle energy gap (�1.5–2 eV) at the Γ point, thereby being quite different from the narrow or zero gaps of group-IV systems. Specifically, experimental measurements have shown that the BP-based field effect transistor has an on/off ratio of 105 and a carrier mobility at room temperature as large as 103 cm2 /Vs. We note that BP is expected to play an important role in the next-generation of electronic devices [6, 20]. Phosphorene exhibits a puckered structure related to the sp<sup>3</sup> hybridization of (3s, 3px, 3py, 3pz) orbitals. The deformed hexagonal lattice of monolayer BP has four

atoms [26], while the group-IV honeycomb lattice includes two atoms. The low-lying energy dispersions, which are dominated by 3pz orbitals, can be described by a fourband model with complicated multi-hopping integrals [26]. The low-lying energy bands are highly anisotropic, e.g., the linear and parabolic dispersions near the Fermi energy EF, respectively, along the ^ kx and ^ ky directions. The anisotropic behaviors are further reflected in other physical properties, as verified by recent measurements on optical and excitonic spectra [27] as well as transport properties [6, 28].

In this work, we have examined the anisotropic behavior of the static polarizability and shielded potential of an impurity for BP. The calculations for the polarizability were executed at T = 0 K and room temperature (T = 300 K). We treat the buckled BP structure as a 2D sheet in our formalism. Consequently, we present an algebraic expression for the surface response function of a pair of 2D layers with arbitrary separation and which are embedded in dielectric media. We then adapt this result to the case when the layer separation is very small to model a freestanding buckled BP structure.

The outline of the rest of our presentation is as follows. In Section 2, we present the surface response function for a pair of 2D layers embedded in background dielectric media. We then simplify this result for a pair of planar sheets which are infinitesimally close to each other and use this for buckled BP. The tight-binding model Hamiltonian for BP is presented in Section 3. This is employed in our calculations of the energy bands and eigenfunctions. Section 4 is devoted to the calculation of the polarizability and dielectric function of BP showing its temperature dependence and their anisotropic properties as a consequence of its band structure. Impurity shielding by BP is discussed in Section 5 and we summarize our important results in Section 6.

as shown in Figure 1. One of the 2D layers is at the top and the other is encapsulated by materials with dielectric constants ϵ1ð Þ ω , with thickness d1, and ϵ2ð Þ ω , of semiinfinite thickness. Calculation shows that the surface response function is given by

(Color online) Schematic illustration of a hybrid structure consisting of a pair of 2D layers separated by

distance d1. The background materials are labeled by dielectric functions ϵ1ð Þ ω and ϵ2ð Þ ω .

Polarizability and Impurity Screening for Phosphorene DOI: http://dx.doi.org/10.5772/intechopen.81814

<sup>g</sup>ð Þ¼ <sup>q</sup>;<sup>ω</sup> <sup>N</sup> ð Þ <sup>q</sup>;<sup>ω</sup>

<sup>2</sup>d1<sup>q</sup> <sup>q</sup>ϵ0ð Þ� <sup>ϵ</sup>1ð Þ� <sup>ω</sup> <sup>1</sup> <sup>χ</sup> f g <sup>1</sup>ð Þ <sup>q</sup>;<sup>ω</sup> <sup>q</sup>ϵ0ðϵ1ð Þþ <sup>ω</sup> <sup>ϵ</sup>2ð Þ <sup>ω</sup> Þ � <sup>χ</sup> f g <sup>2</sup>ð Þ <sup>q</sup>;<sup>ω</sup> � <sup>q</sup>ϵ0ð Þþ <sup>ϵ</sup>1ð Þþ <sup>ω</sup> <sup>1</sup> <sup>χ</sup> f g <sup>1</sup>ð Þ <sup>q</sup>;<sup>ω</sup> <sup>q</sup>ϵ0ðϵ1ð Þ� <sup>ω</sup> <sup>ϵ</sup>2ð Þ <sup>ω</sup> Þ þ <sup>χ</sup> f g <sup>2</sup>ð Þ <sup>q</sup>;<sup>ω</sup> , (4)

f g qϵ0ð Þ� ϵ1ð Þþ ω 1 X1ð Þ q;ω f g qϵ0ðϵ1ð Þþ ω ϵ2ð Þ ω Þ � X2ð Þ q;ω �f g <sup>q</sup>ϵ0ð Þþ <sup>ϵ</sup>1ð Þ� <sup>ω</sup> <sup>1</sup> <sup>X</sup>1ð Þ <sup>q</sup>;<sup>ω</sup> f g <sup>q</sup>ϵ0ðϵ1ð Þ� <sup>ω</sup> <sup>ϵ</sup>2ð Þ <sup>ω</sup> Þ þ <sup>X</sup>2ð Þ <sup>q</sup>;<sup>ω</sup> : (5)

> <sup>2</sup> � <sup>χ</sup>1ð Þþ <sup>q</sup>; <sup>ω</sup> <sup>χ</sup>2ð Þ <sup>q</sup>; <sup>ω</sup> 2qϵ<sup>0</sup>

In this notation, q is the in-plane wave vector, ω is the frequency and χ1ð Þ q;ω

When we take the limit d<sup>1</sup> ! 0, i.e., the separation between the two layer is small, the ϵ<sup>1</sup> drops out and we have the following result for the surface response

Here, the dispersion equation which is given by the zeros of the denominator ϵð Þ q;ω of the second term is expressed in terms of the 'average'susceptibility for the two layers. Clearly, this dispersion equation is that for a 2D layer of the Stern form where we make the identification <sup>χ</sup> ! <sup>e</sup><sup>2</sup>Πð Þ <sup>0</sup> in terms of the polarizability. This

<sup>g</sup>ð Þ¼ <sup>q</sup>;<sup>ω</sup> <sup>1</sup> � <sup>1</sup> 1þϵ2ð Þ ω

<sup>D</sup>ð Þ <sup>q</sup>;<sup>ω</sup> , (3)

: (6)

[29, 30].

Figure 1.

where

and

53

N ð Þ� q;ω e

Dð Þ� q;ω e

2d1q

and χ2ð Þ q;ω are the 2D layer susceptibilities.

function corresponding to the structure in Figure 2

### 2. Surface response function for a pair of 2D layers

Let us consider a heterostructure whose surface is in the xy-plane and suppose that r<sup>∥</sup> denotes the corresponding in-plane translation vector. At time t, an external potential <sup>ϕ</sup>~extð Þ <sup>q</sup>;<sup>ω</sup> with wave vector <sup>q</sup> and frequency <sup>ω</sup> will give rise to an induced potential which, outside the structure, can be written as

$$\phi\_{ind}\left(\mathbf{r}\_{\parallel},t\right) = -\int \frac{d^2\mathbf{q}}{\left(2\pi\right)^2} \int\_{-\infty}^{\infty} d\alpha \tilde{\phi}\_{ext}(q,\alpha) e^{i\left(\mathbf{q}\cdot\mathbf{r}\_{\parallel} - \alpha t\right)} \mathbf{g}(\mathbf{q},\alpha) e^{-qz}.\tag{1}$$

This equation defines the surface response function gð Þ q;ω . It has been implicitly assumed that the external potential ϕext is so weak that the medium responds linearly to it.

The quantity Im[g(q,ωÞ] can be identified with the power absorption in the structure due to electron excitation induced by the external potential. The total potential in the vicinity of the surface (z ≈ 0), is given by

$$\phi(\mathbf{r}\_{\parallel},t) = \int \frac{d^2 \mathbf{q}}{(2\pi)^2} \int\_{-\infty}^{\infty} d\alpha (e^{qx} - \mathbf{g}(\mathbf{q},\omega)e^{-qx})e^{i\left(\mathbf{q}\cdot\mathbf{r}\_{\parallel} - \alpha t\right)} \tilde{\phi}\_{ext}(\mathbf{q},\omega) \tag{2}$$

which takes account of nonlocal screening of the external potential.

#### 2.1 Model for phosphorene layer

In this section, we present the surface response function we calculated for a structure which consists of a pair of 2D layers in contact with a dielectric medium, Polarizability and Impurity Screening for Phosphorene DOI: http://dx.doi.org/10.5772/intechopen.81814

#### Figure 1.

atoms [26], while the group-IV honeycomb lattice includes two atoms. The low-lying energy dispersions, which are dominated by 3pz orbitals, can be described by a fourband model with complicated multi-hopping integrals [26]. The low-lying energy bands are highly anisotropic, e.g., the linear and parabolic dispersions near the Fermi

further reflected in other physical properties, as verified by recent measurements on

In this work, we have examined the anisotropic behavior of the static polarizability and shielded potential of an impurity for BP. The calculations for the polarizability were executed at T = 0 K and room temperature (T = 300 K). We treat the buckled BP structure as a 2D sheet in our formalism. Consequently, we present an algebraic expression for the surface response function of a pair of 2D layers with arbitrary separation and which are embedded in dielectric media. We then adapt this result to the case when the layer separation is very small to model a free-

The outline of the rest of our presentation is as follows. In Section 2, we present

Let us consider a heterostructure whose surface is in the xy-plane and suppose that r<sup>∥</sup> denotes the corresponding in-plane translation vector. At time t, an external potential <sup>ϕ</sup>~extð Þ <sup>q</sup>;<sup>ω</sup> with wave vector <sup>q</sup> and frequency <sup>ω</sup> will give rise to an induced

<sup>d</sup>ωϕ~extð Þ <sup>q</sup>;<sup>ω</sup> <sup>e</sup>

This equation defines the surface response function gð Þ q;ω . It has been implicitly assumed that the external potential ϕext is so weak that the medium responds

The quantity Im[g(q,ωÞ] can be identified with the power absorption in the structure due to electron excitation induced by the external potential. The total

> qz � <sup>g</sup>ð Þ <sup>q</sup>;<sup>ω</sup> <sup>e</sup> �qz ð Þ<sup>e</sup>

In this section, we present the surface response function we calculated for a structure which consists of a pair of 2D layers in contact with a dielectric medium,

<sup>i</sup>ð Þ <sup>q</sup>�r∥�ω<sup>t</sup> <sup>g</sup>ð Þ <sup>q</sup>;<sup>ω</sup> <sup>e</sup>

<sup>i</sup>ð Þ <sup>q</sup>�r∥�ω<sup>t</sup> <sup>ϕ</sup>~extð Þ <sup>q</sup>;<sup>ω</sup> (2)

�qz: (1)

the surface response function for a pair of 2D layers embedded in background dielectric media. We then simplify this result for a pair of planar sheets which are infinitesimally close to each other and use this for buckled BP. The tight-binding model Hamiltonian for BP is presented in Section 3. This is employed in our calculations of the energy bands and eigenfunctions. Section 4 is devoted to the calculation of the polarizability and dielectric function of BP showing its temperature dependence and their anisotropic properties as a consequence of its band structure. Impurity shielding by BP is discussed in Section 5 and we summarize our important

2. Surface response function for a pair of 2D layers

potential which, outside the structure, can be written as

Z d<sup>2</sup> q ð Þ <sup>2</sup><sup>π</sup> <sup>2</sup>

potential in the vicinity of the surface (z ≈ 0), is given by

Z <sup>∞</sup> �∞

dω e

which takes account of nonlocal screening of the external potential.

Z <sup>∞</sup> �∞

<sup>ϕ</sup>ind <sup>r</sup>∥; <sup>t</sup> � � ¼ �

Z d<sup>2</sup> q ð Þ <sup>2</sup><sup>π</sup> <sup>2</sup> ky directions. The anisotropic behaviors are

kx and ^

optical and excitonic spectra [27] as well as transport properties [6, 28].

energy EF, respectively, along the ^

2D Materials

standing buckled BP structure.

results in Section 6.

linearly to it.

52

<sup>ϕ</sup> <sup>r</sup>∥; <sup>t</sup> � � <sup>¼</sup>

2.1 Model for phosphorene layer

(Color online) Schematic illustration of a hybrid structure consisting of a pair of 2D layers separated by distance d1. The background materials are labeled by dielectric functions ϵ1ð Þ ω and ϵ2ð Þ ω .

as shown in Figure 1. One of the 2D layers is at the top and the other is encapsulated by materials with dielectric constants ϵ1ð Þ ω , with thickness d1, and ϵ2ð Þ ω , of semiinfinite thickness. Calculation shows that the surface response function is given by [29, 30].

$$\mathbf{g}(\mathbf{q}, \boldsymbol{\alpha}) = \frac{\mathcal{N}(\mathbf{q}, \boldsymbol{\alpha})}{\mathcal{D}(\mathbf{q}, \boldsymbol{\alpha})},\tag{3}$$

where

$$\mathcal{N}(\mathbf{q},\boldsymbol{\omega}) \equiv \epsilon^{2d \cdot q} \{ q\epsilon\_0(\epsilon\_1(\boldsymbol{\omega}) - \mathbf{1}) - \chi\_1(\mathbf{q},\boldsymbol{\omega}) \} \{ q\epsilon\_0(\epsilon\_1(\boldsymbol{\omega}) + \epsilon\_2(\boldsymbol{\omega})) - \chi\_2(\mathbf{q},\boldsymbol{\omega}) \} \tag{4}$$
 
$$ - \{ q\epsilon\_0(\epsilon\_1(\boldsymbol{\omega}) + \mathbf{1}) + \chi\_1(\mathbf{q},\boldsymbol{\omega}) \} \{ q\epsilon\_0(\epsilon\_1(\boldsymbol{\omega}) - \epsilon\_2(\boldsymbol{\omega})) + \chi\_2(\mathbf{q},\boldsymbol{\omega}) \},$$

and

$$\mathcal{D}(\mathbf{q},\boldsymbol{\omega}) \equiv \boldsymbol{\varepsilon}^{\mathsf{Z}d,q} \{ q\epsilon\_0(\epsilon\_1(\boldsymbol{\alpha}) + \mathbf{1}) - \mathcal{X}\_1(\mathbf{q},\boldsymbol{\omega}) \} \{ q\epsilon\_0(\epsilon\_1(\boldsymbol{\alpha}) + \epsilon\_2(\boldsymbol{\alpha})) - \mathcal{X}\_2(\mathbf{q},\boldsymbol{\omega}) \} \tag{5}$$
 
$$ - \{ q\epsilon\_0(\epsilon\_1(\boldsymbol{\alpha}) - \mathbf{1}) + \mathcal{X}\_1(\mathbf{q},\boldsymbol{\omega}) \} \{ q\epsilon\_0(\epsilon\_1(\boldsymbol{\alpha}) - \epsilon\_2(\boldsymbol{\alpha})) + \mathcal{X}\_2(\mathbf{q},\boldsymbol{\omega}) \}.$$

In this notation, q is the in-plane wave vector, ω is the frequency and χ1ð Þ q;ω and χ2ð Þ q;ω are the 2D layer susceptibilities.

When we take the limit d<sup>1</sup> ! 0, i.e., the separation between the two layer is small, the ϵ<sup>1</sup> drops out and we have the following result for the surface response function corresponding to the structure in Figure 2

$$\log(\mathbf{q}, \boldsymbol{\alpha}) = \mathbf{1} - \frac{\mathbf{1}}{\frac{1 + e\_2(\boldsymbol{\alpha})}{2} - \frac{\chi\_1(\mathbf{q}, \boldsymbol{\alpha}) + \chi\_2(\mathbf{q}, \boldsymbol{\alpha})}{2qe\_0}}} \,. \tag{6}$$

Here, the dispersion equation which is given by the zeros of the denominator ϵð Þ q;ω of the second term is expressed in terms of the 'average'susceptibility for the two layers. Clearly, this dispersion equation is that for a 2D layer of the Stern form where we make the identification <sup>χ</sup> ! <sup>e</sup><sup>2</sup>Πð Þ <sup>0</sup> in terms of the polarizability. This

Our calculation can easily be generalized to the case when the monolayer is embedded above and below by the same thick dielectric material (dielectric constant ϵb) which corresponds to the free-standing situation which we consider below. For this, we have <sup>ϵ</sup>ð Þ¼ <sup>q</sup>;<sup>ω</sup> <sup>ϵ</sup><sup>b</sup> � <sup>e</sup>2=ð Þ <sup>2</sup>ϵ0<sup>q</sup> <sup>Π</sup>ð Þ <sup>0</sup> ð Þ <sup>q</sup>;<sup>ω</sup> , expressed in terms of the 2D layer

Phosphorene is treated as a single layer of phosphorus atoms arranged in a puckered orthorhombic lattice, as shown in Figure 3(a). It contains two atomic layers of A and B atoms and two kinds of bonds for in-plane and inter-plane P–P connections with different bond lengths. The low-lying electronic structure can be described by a tight-binding Hamiltonian, which is a 4 � 4 matrix within the basis

<sup>3</sup> <sup>T</sup><sup>4</sup> <sup>T</sup><sup>2</sup>� <sup>þ</sup> <sup>T</sup><sup>∗</sup>

<sup>1</sup> þ T<sup>3</sup> 0

<sup>2</sup><sup>þ</sup> <sup>þ</sup> <sup>T</sup><sup>5</sup><sup>þ</sup> <sup>0</sup> <sup>T</sup><sup>1</sup> <sup>þ</sup> <sup>T</sup><sup>∗</sup>

Here, we consider up to five nearest atomic interactions through five independent terms of Ti with i ¼ 1; 2; 3; 4; 5. These terms are given by the following expressions.

> ik� d4þþþ d4þ� ! þ d4�þ ! <sup>þ</sup> <sup>d</sup>4�� � �

the atomic interactions. They have been optimized as (t<sup>1</sup> ¼ �1:220, t<sup>2</sup> ¼ 3:665, t<sup>3</sup> ¼ �0:205, t<sup>4</sup> ¼ �0:105, t<sup>5</sup> ¼ �0:055) in order to reproduce the energy bands obtained by the density functional theory (DFT) calculations [31–33]. Also, dm�

d<sup>1</sup>� ¼ ð Þ b=2 � c; � a=2; 0

d<sup>3</sup>� ¼ ð Þ b=2 þ c; � a=2; 0 d<sup>4</sup>� ¼ �ð Þ b=2; � a=2; h d<sup>5</sup>� ¼ �f g ð Þ b � c ; 0; �h ,

where a ¼ 3:314Å, b ¼ 4:376Å, c ¼ 0:705Å, and h ¼ 2:131Å are the distances

The valence and conduction energy bands present strong anisotropic behaviors, as illustrated by the energy bands in Figure 3(b) and the constant-energy loops in Figure 3(c) and (d). As a result, the polarizability and dielectric function are shown

d<sup>2</sup>� ¼ �ð Þ c; 0; h

to be strongly dependent on the direction of the transferred momentum q.

In this notation, tm (m ¼ 1; 2; 3; 4; 5) are the hopping integrals, corresponding to

<sup>5</sup><sup>þ</sup> T<sup>4</sup>

5�

(7)

! are

(8)

3

<sup>0</sup> <sup>T</sup><sup>1</sup> <sup>þ</sup> <sup>T</sup><sup>∗</sup>

<sup>2</sup>� <sup>þ</sup> <sup>T</sup><sup>5</sup>� <sup>T</sup><sup>4</sup> <sup>T</sup><sup>∗</sup>

<sup>T</sup><sup>1</sup> <sup>¼</sup> <sup>t</sup>1e<sup>i</sup>k�ð Þ <sup>d</sup>1þþ <sup>d</sup>1� <sup>T</sup><sup>2</sup>� <sup>¼</sup> <sup>t</sup>2e<sup>i</sup>k�d2� <sup>T</sup><sup>3</sup> <sup>¼</sup> <sup>t</sup>3eik�ð Þ <sup>d</sup>3þþ <sup>d</sup>3�

T<sup>4</sup> ¼ t4e

<sup>T</sup><sup>5</sup>� <sup>¼</sup> <sup>t</sup>5e<sup>i</sup>k�d5� :

the vectors connecting the lattice sites which can be written as

8

>>>>>>>><

>>>>>>>>:

55

between the BP atoms [34, 35], as illustrated in Figure 3(a).

T<sup>4</sup> T<sup>∗</sup>

8

>>>>>>>><

>>>>>>>>:

<sup>1</sup> <sup>þ</sup> <sup>T</sup><sup>3</sup> <sup>0</sup> <sup>T</sup><sup>2</sup><sup>þ</sup> <sup>þ</sup> <sup>T</sup><sup>∗</sup>

polarizability <sup>Π</sup>ð Þ <sup>0</sup> ð Þ <sup>q</sup>;<sup>ω</sup> .

3. Model Hamiltonian

(A1, A2, B1, B2), of the form

T∗

Polarizability and Impurity Screening for Phosphorene DOI: http://dx.doi.org/10.5772/intechopen.81814

T∗

#### Figure 2.

(Color online) Schematic representation of a structure consisting of a pair of 2D layers which are infinitesimally close. There is vacuum above the layers and a dielectric below.

#### Figure 3.

(Color online) The (a) top view and side view of crystal structure for BP and (b) its band structure. The constant-energy diagrams are presented for (c) valence and (d) conduction bands. The values of 2 kF for different θ are given in (d).

result in Eq. (6) clearly illustrates that for the buckled BP structure shown in Figure 3, the dielectric function can be treated as that for a single layer whose susceptibility arises from a combination of two rows of atoms making up the layer. Our calculation can easily be generalized to the case when the monolayer is embedded above and below by the same thick dielectric material (dielectric constant ϵb) which corresponds to the free-standing situation which we consider below. For this, we have <sup>ϵ</sup>ð Þ¼ <sup>q</sup>;<sup>ω</sup> <sup>ϵ</sup><sup>b</sup> � <sup>e</sup>2=ð Þ <sup>2</sup>ϵ0<sup>q</sup> <sup>Π</sup>ð Þ <sup>0</sup> ð Þ <sup>q</sup>;<sup>ω</sup> , expressed in terms of the 2D layer polarizability <sup>Π</sup>ð Þ <sup>0</sup> ð Þ <sup>q</sup>;<sup>ω</sup> .

### 3. Model Hamiltonian

Phosphorene is treated as a single layer of phosphorus atoms arranged in a puckered orthorhombic lattice, as shown in Figure 3(a). It contains two atomic layers of A and B atoms and two kinds of bonds for in-plane and inter-plane P–P connections with different bond lengths. The low-lying electronic structure can be described by a tight-binding Hamiltonian, which is a 4 � 4 matrix within the basis (A1, A2, B1, B2), of the form

$$
\begin{bmatrix}
\mathbf{0} & T\_1 + T\_3^\* & T\_4 & T\_{2-} + T\_{5-}^\* \\
T\_1^\* + T\_3 & \mathbf{0} & T\_{2+} + T\_{5+}^\* & T\_4 \\
T\_4 & T\_{2+}^\* + T\_{5+} & \mathbf{0} & T\_1 + T\_3^\* \\
T\_{2-}^\* + T\_{5-} & T\_4 & T\_1^\* + T\_3 & \mathbf{0}
\end{bmatrix}.
$$

Here, we consider up to five nearest atomic interactions through five independent terms of Ti with i ¼ 1; 2; 3; 4; 5. These terms are given by the following expressions.

$$\begin{cases} T\_1 = t\_1 e^{i\mathbf{k} \cdot (\mathbf{d}\_{\mathbf{i}+} + \mathbf{d}\_{\mathbf{i}-})} \\\\ T\_{2\pm} = t\_2 e^{i\mathbf{k} \cdot \mathbf{d}\_{\mathbf{i}\pm}} \\\\ T\_3 = t\_3 e^{i\mathbf{k} \cdot (\mathbf{d}\_{\mathbf{i}+} + \mathbf{d}\_{\mathbf{i}-})} \\\\ T\_4 = t\_4 e^{i\mathbf{k} \cdot \left(\mathbf{d}\_{\mathbf{i}++} + \mathbf{d}\_{\mathbf{i}+-}^\cdot + \mathbf{d}\_{\mathbf{i}-+}^\cdot + \mathbf{d}\_{\mathbf{i}-}\right)} \\\\ T\_{5\pm} = t\_5 e^{i\mathbf{k} \cdot \mathbf{d}\_{5\pm}} \end{cases} \tag{7}$$

In this notation, tm (m ¼ 1; 2; 3; 4; 5) are the hopping integrals, corresponding to the atomic interactions. They have been optimized as (t<sup>1</sup> ¼ �1:220, t<sup>2</sup> ¼ 3:665, t<sup>3</sup> ¼ �0:205, t<sup>4</sup> ¼ �0:105, t<sup>5</sup> ¼ �0:055) in order to reproduce the energy bands obtained by the density functional theory (DFT) calculations [31–33]. Also, dm� ! are the vectors connecting the lattice sites which can be written as

$$\begin{cases} d\_{1\pm} = (b/2 - c, \pm a/2, \mathbf{0}) \\ d\_{2\pm} = (\pm c, \mathbf{0}, h) \\ d\_{3\pm} = (b/2 + c, \pm a/2, \mathbf{0}) \\ d\_{4\pm} = (\pm b/2, \pm a/2, h) \\ d\_{5\pm} = \{\pm (b - c), \mathbf{0}, -h\}, \end{cases} \tag{8}$$

where a ¼ 3:314Å, b ¼ 4:376Å, c ¼ 0:705Å, and h ¼ 2:131Å are the distances between the BP atoms [34, 35], as illustrated in Figure 3(a).

The valence and conduction energy bands present strong anisotropic behaviors, as illustrated by the energy bands in Figure 3(b) and the constant-energy loops in Figure 3(c) and (d). As a result, the polarizability and dielectric function are shown to be strongly dependent on the direction of the transferred momentum q.

result in Eq. (6) clearly illustrates that for the buckled BP structure shown in Figure 3, the dielectric function can be treated as that for a single layer whose susceptibility arises from a combination of two rows of atoms making up the layer.

(Color online) The (a) top view and side view of crystal structure for BP and (b) its band structure. The constant-energy diagrams are presented for (c) valence and (d) conduction bands. The values of 2 kF for

(Color online) Schematic representation of a structure consisting of a pair of 2D layers which are infinitesimally

close. There is vacuum above the layers and a dielectric below.

Figure 2.

2D Materials

Figure 3.

54

different θ are given in (d).

#### 4. Dielectric function

When monolayer BP is perturbed by an external time-dependent Coulomb potential, all the valence and conduction electrons will screen this field and therefore create the charge redistribution. The effective potential between two charges is the sum of the external potential and the induced potential due to screening charges. The dynamical dielectric function, within the random-phase approximation (RPA), is given by [36].

and higher (q ≥ 0:7 1=Å � �) transferred momentum remains unchanged. In general, <sup>Π</sup>ð Þ <sup>0</sup> ð Þ <sup>0</sup>; <sup>q</sup> falls off rapidly beyond a critical value of <sup>q</sup> (2kF) which depends on <sup>θ</sup>. For increasing θ from 0 to 90°, the specific values are getting larger, as shown in Figure 4(a). This means that the polarizability is stronger for 0.2 ≤ q ≤ 0.7 (1=Å). The main features of the polarizability for BP are quite similar to those for the 2D electron gas, but different with those for graphene. Temperature has an effect on the polarization function which is demonstrated in Figure 4(b). At room temperature, <sup>Π</sup>ð Þ <sup>0</sup> ð Þ <sup>0</sup>; <sup>q</sup> exhibits a shoulder-like structure near the critical values of <sup>q</sup> instead

Plots of the static dielectric function of BP for various values of θ are presented in Figure 4(c) and (d) at absolute zero and room temperatures, respectively. In the range of 0.2 ≤ q ≤ 0.5 (1=Å), there is a clear dependence of the dielectric function on the direction of the transferred momentum q. The Re ϵð Þ 0; q is higher with the growth of θ. The introduction of finite temperature smoothens the q-dependent Re

Starting with Eq. (2), we obtain the static screening of the potential on the

dθe iqr cos θ

By employing the generalized form of Eq. (6) for free-standing BP in Eq. (10), we have computed the screened impurity potential. The screened potentials for various z0's are shown in Figure 5 at absolute zero temperature and Fermi energy

(Color online) The screened impurity potential in units of <sup>e</sup><sup>2</sup>kF,x=ð Þ <sup>ϵ</sup><sup>s</sup> is plotted as a function of kF,xr<sup>k</sup> for the

<sup>d</sup><sup>θ</sup> <sup>e</sup>iqr cos <sup>θ</sup>�qz<sup>0</sup> <sup>ϵ</sup>ð Þ <sup>q</sup>;<sup>ω</sup> <sup>¼</sup> <sup>0</sup> :

<sup>0</sup>e located at distance z<sup>0</sup> above the

�qz<sup>0</sup>

(10)

½ � 1 � gð Þ q;ω ¼ 0 e

of step-like structure at T = 0.

5. Impurity shielding

<sup>ϕ</sup> <sup>r</sup>∥;<sup>ω</sup> <sup>¼</sup> <sup>0</sup> � � <sup>¼</sup> <sup>Z</sup><sup>∗</sup>

surface of BP as

Figure 5.

57

chosen parameters in the figure.

ϵð Þ 0; q , as shown in Figure 4(d) for T = 30 K.

Polarizability and Impurity Screening for Phosphorene DOI: http://dx.doi.org/10.5772/intechopen.81814

surface at <sup>z</sup> <sup>¼</sup> 0 due to an impurity with charge <sup>Z</sup><sup>∗</sup>

0e 2πϵ<sup>0</sup>

<sup>¼</sup> <sup>Z</sup><sup>∗</sup> 0e 2πϵ<sup>0</sup> Z <sup>∞</sup> 0

Z <sup>∞</sup> 0

dq <sup>Z</sup> <sup>2</sup><sup>π</sup> 0

dq <sup>Z</sup> <sup>2</sup><sup>π</sup> 0

$$\begin{split} \epsilon(\mathbf{q}, \boldsymbol{\omega}) &= \epsilon\_{b} - V\_{q} \sum\_{\substack{\mathbf{s}\_{y} \boldsymbol{s}' = \mathbf{q}, \boldsymbol{\theta} \ \boldsymbol{h}\_{h} \boldsymbol{h}' = \boldsymbol{\epsilon}, \boldsymbol{\nu}}} \sum\_{\mathbf{l} \text{ atBZ}} \int\_{\text{LatBZ}} \frac{\mathbf{d} k\_{x} \mathbf{d} k\_{y}}{\left(2\pi\right)^{2}} |\langle \boldsymbol{s}'; \boldsymbol{h}'; \mathbf{k} + \mathbf{q}| e^{i\mathbf{q} \cdot \mathbf{r}} | \boldsymbol{s}; \boldsymbol{h}; \mathbf{k}\rangle|^{2} \\ &\times \frac{f\left(E^{\boldsymbol{\epsilon}', \boldsymbol{h}'} (\mathbf{k} + \mathbf{q})\right) - f\left(E^{\boldsymbol{\epsilon}, \boldsymbol{h}} (\mathbf{k})\right)}{E^{\boldsymbol{\epsilon}', \boldsymbol{h}'} (\mathbf{k} + \mathbf{q}) - E^{\boldsymbol{\epsilon}, \boldsymbol{h}} (\mathbf{k}) - (\boldsymbol{\omega} + i\Gamma)}. \end{split} \tag{9}$$

Here, the π-electronic excitations are described in terms of the transferred momentum q and the excitation frequency ω. ϵ<sup>b</sup> ¼ 2:4 the background dielectric constant, Vq <sup>¼</sup> <sup>2</sup>πe<sup>2</sup>=ð Þ <sup>ε</sup>sq the 2D Fourier transform of the bare Coulomb potential energy (ε<sup>s</sup> ¼ 4πϵ0), and Γ the energy width due to various de-excitation mechanisms. f Eð Þ¼ 1=f g 1 þ exp ½ � ð Þ E � μ kBT the Fermi-Dirac distribution in which kB is the Boltzmann constant and μ the chemical potential corresponding to the highest occupied state energy (middle energy of band gap) in the (semiconducting) metallic systems at T = 0 K.

Figure 4(a) and (b) shows the directional/θ-dependence of the static polarization function <sup>Π</sup>ð Þ <sup>0</sup> ð Þ <sup>0</sup>; <sup>q</sup> , in which <sup>θ</sup> defines the angle between the direction of <sup>q</sup> and the unit vector ^ ky. For arbitrary θ, the polarization function at lower (q ≤ 0:2 1=Å � �)

#### Figure 4.

(Color online) The static polarizability for BP as a function of wave vector for different directions of the transferred momentum q at (a) absolute zero and (b) room temperatures. Plots (c) and (d) correspond to the static dielectric function of BP at T = 0 and 300 K, respectively.

Polarizability and Impurity Screening for Phosphorene DOI: http://dx.doi.org/10.5772/intechopen.81814

and higher (q ≥ 0:7 1=Å � �) transferred momentum remains unchanged. In general, <sup>Π</sup>ð Þ <sup>0</sup> ð Þ <sup>0</sup>; <sup>q</sup> falls off rapidly beyond a critical value of <sup>q</sup> (2kF) which depends on <sup>θ</sup>. For increasing θ from 0 to 90°, the specific values are getting larger, as shown in Figure 4(a). This means that the polarizability is stronger for 0.2 ≤ q ≤ 0.7 (1=Å). The main features of the polarizability for BP are quite similar to those for the 2D electron gas, but different with those for graphene. Temperature has an effect on the polarization function which is demonstrated in Figure 4(b). At room temperature, <sup>Π</sup>ð Þ <sup>0</sup> ð Þ <sup>0</sup>; <sup>q</sup> exhibits a shoulder-like structure near the critical values of <sup>q</sup> instead of step-like structure at T = 0.

Plots of the static dielectric function of BP for various values of θ are presented in Figure 4(c) and (d) at absolute zero and room temperatures, respectively. In the range of 0.2 ≤ q ≤ 0.5 (1=Å), there is a clear dependence of the dielectric function on the direction of the transferred momentum q. The Re ϵð Þ 0; q is higher with the growth of θ. The introduction of finite temperature smoothens the q-dependent Re ϵð Þ 0; q , as shown in Figure 4(d) for T = 30 K.

### 5. Impurity shielding

4. Dielectric function

2D Materials

tion (RPA), is given by [36].

<sup>ϵ</sup>ð Þ¼ <sup>q</sup>;<sup>ω</sup> <sup>ϵ</sup><sup>b</sup> � Vq <sup>∑</sup>s, <sup>s</sup><sup>0</sup>

f Es 0 ,h<sup>0</sup>

�

lic systems at T = 0 K.

the unit vector ^

Figure 4.

56

Es0 ,h<sup>0</sup> <sup>¼</sup><sup>α</sup>, <sup>β</sup>

ð Þ k þ q � �

∑ h, h<sup>0</sup> <sup>¼</sup>c, <sup>v</sup> Z

ð Þ� <sup>k</sup> <sup>þ</sup> <sup>q</sup> Es,hð Þ� <sup>k</sup> ð Þ <sup>ω</sup> <sup>þ</sup> <sup>i</sup><sup>Γ</sup> :

1stBZ

� f Es,hð Þ <sup>k</sup> � �

Here, the π-electronic excitations are described in terms of the transferred momentum q and the excitation frequency ω. ϵ<sup>b</sup> ¼ 2:4 the background dielectric constant, Vq <sup>¼</sup> <sup>2</sup>πe<sup>2</sup>=ð Þ <sup>ε</sup>sq the 2D Fourier transform of the bare Coulomb potential energy (ε<sup>s</sup> ¼ 4πϵ0), and Γ the energy width due to various de-excitation mechanisms. f Eð Þ¼ 1=f g 1 þ exp ½ � ð Þ E � μ kBT the Fermi-Dirac distribution in which kB is the Boltzmann constant and μ the chemical potential corresponding to the highest occupied state energy (middle energy of band gap) in the (semiconducting) metal-

Figure 4(a) and (b) shows the directional/θ-dependence of the static polarization function <sup>Π</sup>ð Þ <sup>0</sup> ð Þ <sup>0</sup>; <sup>q</sup> , in which <sup>θ</sup> defines the angle between the direction of <sup>q</sup> and

(Color online) The static polarizability for BP as a function of wave vector for different directions of the transferred momentum q at (a) absolute zero and (b) room temperatures. Plots (c) and (d) correspond to the

static dielectric function of BP at T = 0 and 300 K, respectively.

ky. For arbitrary θ, the polarization function at lower (q ≤ 0:2 1=Å � �)

dkxdky ð Þ <sup>2</sup><sup>π</sup> <sup>2</sup> <sup>∣</sup>〈<sup>s</sup>

0 ; h<sup>0</sup> ; <sup>k</sup> <sup>þ</sup> <sup>q</sup>∣eiq�r<sup>∥</sup> j j <sup>s</sup>; <sup>h</sup>; <sup>k</sup>〉 <sup>2</sup>

(9)

When monolayer BP is perturbed by an external time-dependent Coulomb potential, all the valence and conduction electrons will screen this field and therefore create the charge redistribution. The effective potential between two charges is the sum of the external potential and the induced potential due to screening charges. The dynamical dielectric function, within the random-phase approxima-

> Starting with Eq. (2), we obtain the static screening of the potential on the surface at <sup>z</sup> <sup>¼</sup> 0 due to an impurity with charge <sup>Z</sup><sup>∗</sup> <sup>0</sup>e located at distance z<sup>0</sup> above the surface of BP as

$$\begin{split} \phi\left(\mathbf{r}\_{\parallel},\boldsymbol{\omega}=\mathbf{0}\right) &= \frac{Z\_{0}^{\*}\boldsymbol{e}}{2\pi\epsilon\_{0}} \int\_{0}^{\infty} dq \int\_{0}^{2\pi} d\theta e^{iqr\cos\theta} [\mathbf{1}-\mathbf{g}\left(\mathbf{q},\boldsymbol{\omega}=\mathbf{0}\right)] e^{-qx\_{0}} \\ &= \frac{Z\_{0}^{\*}\boldsymbol{e}}{2\pi\epsilon\_{0}} \int\_{0}^{\infty} dq \int\_{0}^{2\pi} d\theta \frac{e^{iqr\cos\theta-qx\_{0}}}{\epsilon(\mathbf{q},\boldsymbol{\omega}=\mathbf{0})} .\end{split} \tag{10}$$

By employing the generalized form of Eq. (6) for free-standing BP in Eq. (10), we have computed the screened impurity potential. The screened potentials for various z0's are shown in Figure 5 at absolute zero temperature and Fermi energy

#### Figure 5.

(Color online) The screened impurity potential in units of <sup>e</sup><sup>2</sup>kF,x=ð Þ <sup>ϵ</sup><sup>s</sup> is plotted as a function of kF,xr<sup>k</sup> for the chosen parameters in the figure.

EF = 1.0 eV. There exist Friedel oscillations for sufficiently small z0. Such oscillations might be smeared out for larger z0, e.g., the green and red curves. It is noticed that for EF = 1.0 eV, the room temperature of 300 K which is much smaller than the Fermi temperature (10,000 K) does not have significant effect on the screened potential. Apparently, V r∥; z<sup>0</sup> at T = 0 and 300 K (not shown) are almost equivalent.

### 6. Concluding remarks and summary

The energy band structure of BP, calculated using the tight-binding method, is anisotropic and so are its polarizability, dielectric function and screened potential. To illustrate these facts, we have presented numerical results for the polarizability in the x and y directions for a range of doping concentrations. The Re[ϵð Þ q;ω ¼ 0 ] of the static dielectric function for BP also reveals some interesting characteristics. At absolute zero temperature (T = 0) and with free carrier density corresponding to chosen Fermi energy EF, we have presented numerical results for Re[ϵð Þ q;ω ¼ 0 ] in different directions of the transferred momentum q. When q is larger than a critical value which is twice the Fermi momentum kF, our calculations show that Re [ϵð Þ q;ω ¼ 0 ] becomes substantially dependent on the direction of q. We also discuss the case at room temperature (T = 300 K). These results are in agreement with those reported by other authors. We employ our data to determine the static shielding of an impurity in the vicinity of phosphorene.
