
Research Article Volume 4 Issue 3
A New Nonrelativistic Investigation for Interactions in One-Electron Atoms With Modified Inverse-Square Potential: Noncommutative Two and Three Dimensional Space Phase Solutions at Planck’s and Nano-Scales
Abdelmadjid Maireche
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Department of Physics, University of M'sila M'sila, Algeria
Correspondence: Abdelmadjid Maireche, Laboratory of Physics and Material Chemistry, Physics department, University of M'sila-Msila Algeria, Tel +213664834317
Received: May 30, 2016 | Published: November 28, 2016
Citation: Maireche A (2016) A New Nonrelativistic Investigation for Interactions in One-Electron Atoms With Modified Inverse-Square Potential: Noncommutative Two and Three Dimensional Space Phase Solutions at Planck’s and Nano-Scales. J Nanomed Res 4(3): 00090. DOI: . DOI: 10.15406/jnmr.2016.04.00090
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Abstract
In this paper, we present a novel theoretical analytical perform further investigation for the exact solvability of non–relativistic quantum spectrum systems for modified inverse–square potential (m.i.s.) potential is discussed by means Boopp’s shift method instead to solving deformed Schrödinger equations with star product, in the framework of both noncommutativity (two –three) dimensional real space and phase (NC: 2D–RSP) and (NC: 3D–RSP). The exact corrections for excited states are found straightforwardly for interactions in one–electron atoms by means of the standard perturbation theory. Furthermore, the obtained corrections of energies are depended on four infinitesimals parameters ( , ) and ( , ), which are induced by position–position and momentum–momentum noncommutativity, (NC: 2D–RSP) and (NC: 3D–RSP), respectively, in addition to the discreet atomic quantum numbers: and (the angular momentum quantum number) and we have also shown that, the usual states in ordinary two and three dimensional spaces are cancelled and has been replaced by new degenerated sub–states in the new quantum symmetries of (NC: 2D–RSP) and (NC: 3D–RSP).
Keywords: the inverse–square potential, noncommutative space, phase, star product, boopp’s shift method.
Abbreviations
MIS: Modified Inverse Square potential; NC: 2D–3D–RSP: Noncommutativity (two–three) Dimensional Real Space Phase; CCRs: Canonical Commutations Relations; NNCCRs: New Noncommutative Canonical Commutations Relations; MSE: Modified Schrödinger Equations.
Introduction
It is well–known, that, the modern quantum mechanics, satisfied a big successful in the last few years, for describing atoms, nuclei, and molecules and their spectral behaviors based on three fundamental equations: Schrödinger, Klein–Gordon and Dirac. Schrödinger equation rest the first and the latest in terms of interest, it is playing a crucial role in devising well–behaved physical models in different fields of physics and chemists, many potentials are treated within the framework of nonrelativistic quantum mechanics based on this equation in two, three and D generalized spaces.1–32 the quantum structure based to the ordinary canonical commutations relations (CCRs) in both Schrödinger and Heisenberg (the operators are depended on time) pictures (CCRs), respectively, as:
[xi,pj]=iδij and [xi,xj] = [pi,pj] = 0
.…(1.1)
[xi(t),pj(t)] = iδij and [xi(t),xj(t)] = [pi(t),pj(t)] = 0
… (1.2)
Where the two operators (xi(t),pi(t))
in Heisenberg picture are related to the corresponding two operators (xi,pi)
in Schrödinger picture from the two projections relations:
xi(t)=exp(iH(t−t0))xiexp(−iH(t−t0)) and pi(t)=exp(iH(t−t0))piexp(−iH(t−t0))
…(1.3)
Here denote to the ordinary quantum Hamiltonian operator, recently, much considerable effort has been expanded on the solutions of Schrödinger, Dirac and Klein–Gordon equations to noncommutative quantum mechanics, the present paper investigates first the present new quantum structure which based to new noncommutative canonical commutations relations (NNCCRs) in both Schrödinger and Heisenberg pictures, respectively, as follows.33–60
[ˆxi∗,ˆpj]=iδij,[ˆxi∗,ˆxj]=iθij and [ˆpi∗,ˆpj]=iˉθij[ˆxi(t)∗,ˆpj(t)]=iδij,[ˆxi(t)∗,ˆxj(t)]=iθij and [ˆpi(t)∗,ˆpj(t)]=iˉθij
…. (1.4)
Where the two new operators (ˆxi(t),ˆpi(t))
in Heisenberg picture are related to the corresponding two new operators (ˆxi,ˆpi)
in Schrödinger picture from the two projections relations:
ˆxi(t)=exp(iHnc(t−t0))*ˆxi*exp(−iHnc(t−t0)) and ˆpi(t)=exp(iHnc(t−t0))*ˆpi*exp(−iHnc(t−t0))
(1.5)
Here Hnc
denote to the new quantum Hamiltonian operator in the symmetries of (NC: 2D–RSP) and (NC: 3D–RSP). The very small two parameters θμν
and ˉθμν
(compared to the energy) are elements of two ant symmetric real matrixes and (∗)
denote to the new star product, which is generalized between two arbitrary functions f(x,p)
and g(x,p)
to (f∗g)(x,p)
instead of the usual product (fg)(x,p)
in ordinary (two–three) dimensional spaces.39–63
(f∗g)(x,p) ≡ exp(i2θμν∂xμ∂xν+i2ˉθμν∂pμ ∂pν)(fg)(x,p) = (fg−i2θμν∂xμf∂xνg−i2ˉθμν∂pμf ∂pνg)(x,p)|(xμ=xν,pμ=pν)+O(θ2,ˉθ2)
.(2)
Where the two covariant derivatives (∂xμf(x,p),∂pμf(x,p))
are denotes to the (∂f(x,p)∂xμ,∂f(x,p)∂pμ)
, respectively, and the two following terms [−i2θμν∂xμf(x,p)∂xνg(x,p)
, −i2ˉθμν∂pμf(x,p) ∂pνg(x,p)
] are induced by (space–space) and (phase–phase) noncommutativity properties, respectively, a Boopp's shift method can be used, instead of solving any quantum systems by using directly star product procedure.39–66
[ˆxi,ˆxj]=iθijand[ˆpi,ˆpj]=iˉθij
...(3.1)
The, four generalized positions and momentum coordinates in the noncommutative quantum mechanics (ˆx,ˆy)
and (ˆpx,ˆpy)
are depended with corresponding four usual generalized positions and momentum coordinates in the usual quantum mechanics (x,y)
and (px,py)
by the following four relations.32–55
{ˆx=x−θ2py,ˆy=y+θ2pxˆpx=px+ˉθ2y andˆpy=px−ˉθ2x
…(3.2)
{ˆx=x−θ122py−θ132pz,ˆy=y−θ212px−θ232pzand ˆz=z−θ312px−θ322py
…(3.3)
and
{ˆpx=px−ˉθ122y−ˉθ132z,ˆpy=py−ˉθ212x−ˉθ232zand ˆpz=pz−ˉθ312x−ˉθ322y
…(3.4)
The non–vanish 9–commutators in (NC–2D: RSP) and (NC–3D: RSP) can be determined as follows:
[ˆx,ˆpx]=[ˆy,ˆpy]=i,[ˆx,ˆy]=iθ12 and [ˆpx,ˆpy]=iˉθ12
…(3.5)
and
[ˆx,ˆpx]=[ˆy,ˆpy]=[ˆz,ˆpz]=i,[ˆx,ˆy]=iθ12,[ˆx,ˆz]=iθ13,[ˆy,ˆz]=iθ23[ˆpx,ˆpy]=iˉθ12,[ˆpy,ˆpz]=iˉθ23,[ˆpx,ˆpz]=iˉθ13
….(3.6)
Which allow us to getting the two operators ˆr2
and ˆp2
on a noncommutative two dimensional space–phase as follows.32–48
ˆr2=r2−θLz and ˆp2=p2+ˉθLz
…(4.1)
ˆr2=r2−→L→Θ and ˆp22μ = p22μ + →L→ˉθ2μ
…(4.2)
Where the two couplings LΘ
and are given by, respectively:
LΘ≡LxΘ12+LyΘ23+LzΘ13 and →L→ˉθ≡Lxˉθ12+Lyˉθ23+Lzˉθ13
… (5.1)
It is–well known, that, in quantum mechanics, the three components (Lx
Ly
, Lz
and ) are determined, in Cartesian coordinates:
Lx=ypz−zpy,Ly =zpx-xpz and Lz=xpy−ypx
… (5.2)
The study of inverse–square potential has now become a very interest field due to their applications in different fields.1 this work is aimed at obtaining an analytic expression for the eigenenergies of a inverse–square potential in (NC: 2D–RSP) and (NC: 3D–RSP) using the generalization Boopp’s shift method based on mentioned formalisms on above equations to discover the new symmetries and a possibility to obtain another applications to this potential in different fields, it is important to notice that, this potential was studied, in ordinary two dimensional spaces, by authors Shi–Hai Dong and Guo–Hua Sun of the Ref. the Schrödinger equation with a Coulomb plus inverse–square potential in D dimensions.1 The organization scheme of the study is given as follows: In next section, we briefly review the Schrödinger equation with inverse–square potential on based to Ref.1 The Section 3, devoted to studying the (two–three) deformed Schrödinger equation by applying both Boopp's shift method to the inverse–square potential. In the fourth section and by applying standard perturbation theory we find the quantum spectrum of the excited states in (NC–2D: RSP) and (NC–3D: RSP) for spin–orbital interaction. In the next section, we derive the magnetic spectrum for studied potential. In the sixth section, we resume the global spectrum and corresponding noncommutative Hamiltonian for inverse–square potential. Finally, the important results and the conclusions are discussed in last section.
Review the eignenfunctions and the energy eigenvalues for inverse–square potential in ordinary two dimensional spaces
Here we will firstly describe the essential steps, which gives the solutions of time independent Schrödinger equation for a fermionic particle like electron of rest mass and its energy moving in inverse–square potential.1
V(r)=Ar2−Br
… (6)
Where A and B are two positive constant coefficients. The above potential is the sum of Colombian
(−Br)
and inverse–square potential (Ar2)
, if we insert this potential into the non–relativistic Schrödinger equation; we obtain the following equation, in two and three dimensional spaces, respectively, as follows:
{−ℏ22m0[1r∂∂r(r∂∂r)+1r2∂2∂ϕ2]−Ar2+Br}Ψ(r,ϕ)=Ε2dΨ(r,ϕ)
… (7.1)
{−ℏ22m0[1r2∂∂r(r2∂∂r)+1r2sinθ∂∂θ(sinθ∂∂θ)+1r2(sinθ)2∂2∂ϕ2]−Ar2+Br}Ψ(r,θ,ϕ)=Ε3dΨ(r,θ,ϕ)
…. (7.2)
Here Ψ(r,ϕ)
and Ψ(r,θ,ϕ)
is the solution in the (2–3) dimensional in (polar and spherical) coordinates, the complete wave function ( Ψ(r,ϕ)
and Ψ(r,θ,ϕ)
separated as follows:
Ψ(r,ϕ)=Rl(r)e±iϕ
...(8.1)
and
Ψ(x)=Rl(r)Yll(θ,ϕ)
… (8.2)
Substituting eq. (8.1) and (8.2) into eq. (7.1) and (7.2), we obtain the radial function satisfied the following equation, in (two–three) dimensional spaces.1
d2Rl(ρ)dρ2+2ρdRl(ρ)dρ+(−14+τρ−2A+l2ρ2)Rl(r) = 0
…(9.1)
1r2∂∂r(r2∂∂r)Rl(r)+[2(Ε−V(r))−l(l+1)r2]Rl(r) = 0
… (9.2)
Hereρ=r√−8E
and τ=B√−12E
.
The proposed solutions of eqs. (9.1) and (9.2) are determined from the unifed relation:
R1(ρ)=ρλe−ρ2F(ρ)
(10)
where λ=2−D+√2A+k22
and k=2l+D−2
. We Companie between eqs. (9.1), (9.2) and (10) to obtains.1
ρd2F(ρ)dρ2+(2λ+D−1−ρ)+dF(ρ)dρ+(τ−λ−D−12)F(ρ)=0
…(11)
The confluent hypergeometric functions φ(λ−τ+1/2,2λ+1;ρ)
are present the solutions of eq. (11).1
R(ρ)=Νρλe−ρ2φ(λ−τ+(D−1)/2,2λ+D−1;ρ)
…(12)
The constraint conditions on the potential parameters are determined from relations.1
τ−λ−(D−1)/2=n′=0,1,2,.......n=n′+κ2−D/2+2=n′+l+1τ=Β√1−2Ε=n−l−1+λ+(D−1)/2
… (13)
The normalized wave functions Ψ(ρ,ϕ)
expressed in terms of the radial functions and spherical harmonic functions read as.1
Ψ(ρ,ϕ)=(4Β2n−2m+2s2−1)((n−m−1)!(2n−2m+2s2−1)(n−m+2s2−1)!)1/2ρs2e−ρ2L2s2n−m−1(ρ)exp(±imϕ)
..(14.1)
Ψ(ρ)=(2Bn)32[(n−l−1)!2n(n+l)!]12ρle−ρ2L2l+1n−l−1(ρ)Yll(θ,ϕ)
…(14.2)
And the corresponding eigenvalues Ε(n,l,D)
is determined from relation.1
Ε(n,l,D)=−2Β(2n−2l−1+√8Α+κ2)={−2Β2(2n−2m−1+√2A+m2)2 forD=2−2B2{(2n)−2−8Aκ(2n)−3+16A2κ3(2n)−3+48A2κ2(2n)−4−...} forD=3
(15)
The rest of this section is devoted to the reapply of some essential properties of generalized Laguerre polynomials L(β)n(ρ)
which are given by:
L(β)n(ρ)≡12∏i∮exp(−ρt1−t)(1−t)β+1tn+1dt
…(16)
Where is integer, this can be taking the exciplicitly mathematically forms.1,65,66,67
L(β)n(ρ)=β(β+n+1)n!β(β+1)F11(−n,β+1;ρ)
…(17)
The Laguerre polynomials may be defined in terms of hypergeometric functions 1F1(−n,β+1;ρ)
, specifically the confluent hyper geometric functions, as:
F11(−n,β+1;ρ)=∞∑n=0a(n)ρnb(n)n!
… (18.1)
Where a(n)
is the Pochhammer symbol, which can be takes the particulars values a(0)=0
and a(n)=a(a+1).....(a+n−1)
, it is important to notice that, the hypergeometric functions have another common notation Φ(a,b,ρ)
which considered as a function of a, b=0,−1,−2,...
, and the variable ρ
. The generalized Laguerre polynomial can also be defined by the following equation:
L(β)n(ρ)=n∑i=0(−1)i(n+βn−i)(i)!ρi
…(18.2)
Deformed schrödinger equations and modified inverse–square (m.i.s.) potential in both (nc–2d: rsp) and (nc–3d: rsp):
This section is devoted to constructing of non relativistic modified Schrödinger equations (m.s.e) in both (NC–2D: RSP) and (NC–3D: RSP) for (m.i.s.) potential; to achieve this subject, we apply the essentials following steps.32–48
- Ordinary two dimensional Hamiltonian operators ( ˆHis2(pi,xi)
, ˆHis3(pi,xi)
) will be replaced by new two dimensional Hamiltonian operators (ˆHnc2−is(ˆpi,ˆxi)
, ˆHnc3−is(ˆpi,ˆxi)
),
- Ordinary complex wave function Ψ(→r)
will be replacing by new complex wave function ⌢Ψ(↔⌢r)
,
- Ordinary energies E(n,l,2)
and E(n,l,3)
will be replaced by new values Enc2−is(n,l,2,...)
and Enc3−is(n,l,3,...)
, respectively.
And the last step corresponds to replace the ordinary old product by new star product (∗)
, which allow us to constructing the modified two dimensional Schrödinger equation in both (NC–2D: RSP) and (NC–3D: RSP) as for (m.i.s.) potential:
ˆHnc2−is(ˆpi,ˆxi)∗⌢Ψ(↔⌢r)=Enc2−is(n,l,2,...)⌢Ψ(↔⌢r)
…. (19.1)
and
ˆHnc3−is(ˆpi,ˆxi)∗⌢Ψ(↔⌢r)=Enc3−is(n,l,3,...)⌢Ψ(↔⌢r)
…(19.2)
In order to use the ordinary product without star product, with new vision, as mentioned before, we apply the Boopp’s shift method on the above eqs. (19.1) and (19.2) to obtain two reduced Schrödinger in both (NC–2D: RSP) and (NC–3D: RSP) for (m.i.s.) potential:
Hnc2−is(ˆpi,ˆxi)ψ(→r)=Enc2−is(n,l,2,...)ψ(→r)
.... (20.1)
and
Hnc3−is(ˆpi,ˆxi)ψ(→r)=Enc3−is(n,l,3,...)ψ(→r)
....(20.2)
Where the new operators of Hamiltonian Hnc2−is(∧pi,∧xi)
and Hnc3−is(ˆpi,ˆxi)
can be expressed in three general varieties: both noncommutative space and noncommutative phase (NC–2D: RSP, NC–3D: RSP), only noncommutative space (NC–2D: RS, NC–3D: RS) and only noncommutative phase (NC: 2D–RP, NC: 3D–RP) as, respectively:
Hnc(2−3)−is(ˆpi,ˆxi)≡H(px+ˉθ2y,py−ˉθ2x,x−θ2py,y+θ2px)for NC-2D: RSP and NC-3D: RSP
...(21.1)
Hnc(2−3)−is(ˆpi,ˆxi)≡H(px,py,x−θ2py,y+θ2px) for NC-2D: RS and NC-3D: RS
...(22.2)
Hnc(2−3)−is(ˆpi,ˆxi)≡H(px+ˉθ2y,px−ˉθ2x,x,y) for NC-2D: RP and NC-3D: RP
...(22.3)
In recently work, we are interest with the first variety (21.1), after straightforward calculations, we can obtain the five important terms, which will be use to determine the (m.i.s.) potential in (NC: 2D– RSP) and (NC: 3D–RSP), respectively, as:
Aˆr2=Ar4+AθLzr4, Bˆr=Br−BθLz2r3 and ˆp22m0=p22m0+→L→ˉθ2m0
…(23)
and
Aˆr2=Ar4+A→L→Θr4, Bˆr=Br−B→L→Θ2r3 and ˆp22m0=p22m0+ˉθLz2m0
…(24)
Which allow us to obtaining the global potential operator Hnc2−is(ˆpi,ˆxi)
and Hnc3−is(ˆpi,ˆxi)
for (m.i.s) potential in both (NC: 2D–RSP) and (NC: 3D–RSP), respectively, as:
Hnc2−is(ˆpi,ˆxi)=Ar2−Br+p22m0+ˉθLz2m0+(Ar4−B2r3)θLz
…(25.1)
and
Hnc3−is(ˆpi,ˆxi)=Ar2−Br+p22m0+→L→ˉθ2m0+(Ar4−B2r3)→L→Θ
…(25.2)
It’s clearly, that the four first terms are given the ordinary inverse–square potential and kinetic energy in (2D–3D) spaces, while the rest terms are proportional’s with infinitesimals parameters (θ
, ˉθ
) and (Θ
, ˉθ
), thus, we can considered as a perturbations terms, we noted by ˆH2−pert(r,A,B,θ,ˉθ)
and ˆH3−pert(r,A,B,Θ,ˉθ)
for (NC: 2D–RSP) and (NC: 3D–RSP) symmetries, respectively, as:
ˆH2−pert(r,A,B,θ,ˉθ)=Lzˉθ2m0+(Ar4−B2r3)θLz
…(26.1)
and
ˆH3−pert(r,A,B,Θ,ˉθ)=→L→ˉθ2m0+(Ar4−B2r3)→L→Θ
…(26.2)
The Exact Spin–Orbital Hamiltonian and the Corresponding Spectrum for (m.i.s.) Potential in both (NC: 2D– RSP) and (NC: 3D– RSP) Symmetries for Excited States for One–Electron Atoms
The exact spin–orbital hamiltonian for (m.i.s.) potential in both (NC: 2D– RSP) and (NC: 3D– RSP) symmetries for one–electron atoms
Again, the perturbative two terms ˆH2−pert(r,A,B,θ,ˉθ)
and ˆH3−pert(r,A,B,Θ,ˉθ)
can be rewritten to the equivalent physical form for (m.i.p.) potential:
ˆH2−pert(r,A,B,θ,ˉθ)={ˉθ2m0+θ(Ar4−B2r3)}↔S↔L
… (26.3)
ˆH3−pert(r,A,B,Θ,ˉθ)={ˉθ2m0+Θ(Ar4−B2r3)}↔S↔L
… (26.4)
Furthermore, the above perturbative terms ˆH2−pert(r,A,B,θ,ˉθ)
and ˆH3−pert(r,A,B,Θ,ˉθ)
can be rewritten to the following new equivalent form for (m.i.p.) potential:
∧H2−pert(r,A,B,θ,−θ)=12{−θ2m0+θ(Ar4−B2r3)}(↔J2−↔L2−↔S2)
(27.1)
ˆH3−pert(r,A,B,Θ,ˉθ)=12{ˉθ2m0+Θ(Ar4−B2r3)}(↔J2−↔L2−↔S2)
… (27.2)
To the best of our knowledge, we just replace the coupling spin–orbital ↔S↔L
by the expression 12(↔J2−↔L2−↔S2)
, in quantum mechanics. The set ( Hnc(2−3)−is(ˆpi,ˆxi)
,J2
, L2
, S2
and Jz)
forms a complete of conserved physics quantities and the eigenvalues of the spin orbital coupling operator are:
p±(j=l±1/2,l,s=1/2)≡12{(l+12)(l+12+1)+l(l+1)−34 ≡ p+ forj= l+12⇒polarization−up(l−12)(l−12+1)+l(l+1)−34 ≡ p− forj= l+12⇒polarization−down
… (27.3)
Which allows us to form a diagonal (2×2)
and (3×3)
two matrixes, with non null elements are [(ˆHso−is)11
and (ˆHso−is)22
] and [(ˆHso−is)11
,(ˆHso−is)22
, (ˆHso−is)33
] for (m.i.s.) potential in (NC: 2D–RSP) and (NC: 3D–RSP), respectively, as:
(Hso−ip)11=p+(ˉθ2m0+θ(Ar4−B2r3)) if j=l+12 ⇒spin -up(Hso−ip)22=p−(ˉθ2m0+θ(Ar4−B2r3)) if j=l−12 ⇒spin -down
....(28.1)
and
(ˆHso−is)11=p+{ˉθ2m0+Θ(Ar4−B2r3)} if j=l+12 ⇒spin up(ˆHso−is)22= p−{ˉθ2m0+Θ(Ar4−B2r3)} ifj = l−12 ⇒spin down(ˆHso−is)33=0
…(28.2)
Substituting two equations (26.1) and (26.2) into two equations (20.1) and (20.12), respectively and then, the radial parts of the modified Schrödinger equations, satisfying the following important two equations:
d2Rl(ρ)dρ2+2ρdRl(ρ)dρ+(−14+τρ−2A+l2ρ2−{ˉθ2m0+θ(Ar4−B2r3)}↔S↔L)Rl(r) = 0
… (29.1)
and
1r2∂∂r(r2∂∂r)Rl(r)+[2(Enc3−is(n,l,3,...)−V(r))−l(l+1)r2−{ˉθ2m0+Θ(Ar4−B2r3)}↔S↔L]Rl(r)=0
…(29.2)
for (m.i.s.) potential in (NC: 2D–RSP) and (NC: 3D–RSP), ii is clearly that the above equations including equations (26.1) and (26.2), the perturbative terms of Hamiltonian operator, which we are subject of discussion in next sub–section.
The exact spin–orbital spectrum for (m.i.s.) potential in both (NC: 2D– RSP) and (NC: 3D– RSP) symmetries for states for one–electron atoms
In this sub section, we are going to study the modifications to the energy levels (Enc−per:u(θ,ˉθ)
,Enc−per:D(θ,ˉθ)
) and (Enc−per:u(Θ,ˉθ)
, Enc−per:D(Θ,ˉθ)
) for spin up and spin down, respectively, at first order of parameters (θ
,ˉθ
) and ( Θ
, ˉθ
), for excited states nth
, obtained by applying the standard perturbation theory, using eqs. (14.1) (14.2), (27.1) and (27.2) corresponding (NC–2D: RSP) and (NC–3D: RSP), respectively, as:
Enc−per:u(θ,ˉθ)≡2∏p+∫R*(r)[θ(Ar4−B2r3)+ˉθ2m0]R(r)rdr Sij=l+12Enc−per:D(θ,ˉθ)≡2∏p−∫R*(r)[θ(Ar4−B2r3)+ˉθ2m0]R(r)rdr Sij=l−12
… (30.1)
and
Enc−per:u(Θ,ˉθ)≡−αp+(−8E)3/2(2Bn)3(n−l−1)!2n(n+l)!∫ρ2l+2e−ρ[L2l+1n−l−1(ρ)]2[Θ(A'
….(30.2)
A direct simplification gives:
...(31.1)
and
…(32.2)
Where, the 6– terms: (
,
),
and
are given by:
….(33.1)
and
….(33.2)
With new notation
and
, know we apply the special integral.1, 61
…(34)
,
can be takes: ( -3, –2 and +1),
and
, which allow us to obtaining in (NC: 2D–RSP):
....(35.1)
...(35.2)
....(35.3)
For (NC: 3D–RSP) symmetries, we have:
...(36.1)
...(36.2)
...(36.3)
Which allow us to obtaining the exact modifications of fundamental states (
,
) and (
,
) produced by spin–orbital effect:
…(37.1)
and
....(37.2)
Where, the two factors
and
are given by, respectively:
...(38)
The exact magnetic spectrum for (m.i.s.) potential in both (NC: 2D– RSP) and (NC: 3D– RSP) symmetries for excited states for one–electron atoms
Having obtained the exact modifications to the energy levels (
,
) and (
,
), for exited
states, produced with spin–orbital induced Hamiltonians operators, we now consider interested physically meaningful phenomena, which produced from the perturbative terms of inverse–square potential related to the influence of an external uniform magnetic field, it’s sufficient to apply the following three replacements to describing these phenomena:
.....(39.1)
..(39.2)
....(39.3)
Here
and
are infinitesimal real proportional’s constants, and we choose the magnetic field
, which allow us to introduce the modified new magnetic Hamiltonians
and
in (NC: 2D–RSP) and (NC: 3D–RSP), respectively, as:
....(40.1)
and
....(40.2)
Here
denote to the ordinary Hamiltonian of Zeeman Effect. To obtain the exact noncommutative magnetic modifications of energy (
,
) for modified inverse–square potential, which produced automatically by the effect of
and
, we make the following three simultaneously replacements:
....(41)
In two Eqs. (37.1) and (37.2) to obtain the two values
and
for the exact magnetic modifications of spectrum corresponding
excited states, in (NC–2D: RSP) and (NC–3D: RSP), respectively, as:
...(42.1)
and
....(42.2)
Where
denote to the angular momentum quantum number,
, which allow us to fixing (
) values for the orbital angular momentum quantum numbers.
Results of exact modified global spectrum of the lowest excitations states for (m.i.s.) potential in both (nc:2d– rsp) and (nc:3d– rsp) symmetries for one–electron atoms
Let us now resume the eigenenergies of the modified Schrödinger equations obtained in this paper, the total modified energies (
,
) and (
,
) of a particle fermionic with spin up and spin down are determined corresponding excited states, respectively, for modified inverse–square potential in (NC: 2D–RSP) and (NC: 3D–RSP), on based to the obtained new results (10.a), (37.1), (37.2), (41.1), (41.2) and (37.b), in addition to the original results (17) of energies we obtain the four new values of global energies:
.....(43.1)
...(43.2)
.....(43.3)
....(43.3)
In this way, one can obtain the complete energy spectra for (m.i.s.) potential in (NC: 2D–RSP) and (NC: 3D–RSP) symmetries. Know the following accompanying constraint relations:
- The original spectrum contain two possible values of energies in ordinary two–three dimensional space which presented by equation (15),
- The quantum number m satisfied the interval:
, thus we have (
) values for this quantum number,
- We have also two values for
and
.
Allow us to deduce the important original results: every state in usually (two–three) dimensional space will be replace by
sub–states and then the degenerated state can be take
values in (NC: 2D–RSP) and (NC: 3D–RSP) symmetries. It’s clearly, that the obtained eigenvalues of energies are real and then the noncommutative diagonal Hamiltonian operators
and
are Hermitian, furthermore it’s possible to writing the two elements [
,
] and
, as follows, respectively:
....(44.1)
and
....(44.2)
On the other hand, the above obtain results (44.1) and (44.2) allow us to constructing the diagonal anisotropic matrixes
and
of the Hamiltonian operators
and
for (m.i.s.) potential in (NC: 2D–RSP) and (NC: 3D–RSP) symmetries respectively, as:
...(45.1)
and
...(45.2)
Which allows us to obtain the original results for this investigation: the obtained Hamiltonian operators (45.1) and (45.2) can be describing atom which has two permanent dipoles: the first is electric dipole moment and the second is magnetic moment in external stationary electromagnetic field. It is important to notice that, the appearance of the polarization states of a fermionic particle for (m.i.s.) potential indicate to the validity of obtained results at very high energy where the two relativistic equations: Klein–Gordon and Dirac will be applied, which allowing to apply these results of various Nano–particles at Nano scales.
Conclusion
In this study we have performed the exact analytical bound state solutions: the energy spectra and the corresponding noncommutative Hamiltonians for the two and three dimensional Schrödinger equations in polar and spherical coordinates for modified inverse–squire potential by using generalization Boopp’s Shift method and standard perturbation theory. It is found that the energy eigenvalues depend on the dimensionality of the problem and new atomic quantum numbers (
and the angular momentum quantum number in addition to two infinitesimals parameters (
,
) and (
,
) in the symmetries of (NC: 2D–RSP) and (NC: 3D–RSP). And we also showed that the obtained energy spectra degenerate and every old state will be replaced by
sub–states. Finally, we expect that the results of our research are valid in the high energies, thus the (m.s.e) can gives the same results of Dirac and Klein–Gordon equations.
Acknowledgments
This work was supported with search laboratory of: Physique et Chimie des matériaux, in university of M'sila, Algeria.
Conflicts of interest
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