Helium atom

A helium atom is an atom of the chemical element helium. Helium is composed of two electrons bound by the electromagnetic force to a nucleus containing two protons along with either one or two neutrons, depending on the isotope, held together by the strong force. Unlike for hydrogen, a closed-form solution to the Schrödinger equation for the helium atom has not been found. However, various approximations, such as the Hartree–Fock method, can be used to estimate the ground state energy and wavefunction of the atom.

This article is about the physics of atomic helium. For other properties of helium, see Helium.

Helium atom

Helium-4
Names
Systematic IUPAC name Helium[1]
Identifiers
CAS Number	7440-59-7^Y
3D model (JSmol)	Interactive image
ChEBI	CHEBI:33681^Y
ChemSpider	22423^Y
EC Number	231-168-5
Gmelin Reference	16294
KEGG	D04420^N
MeSH	Helium
PubChem CID	23987
RTECS number	MH6520000
UNII	206GF3GB41^Y
UN number	1046
InChI InChI=1S/He^Y Key: SWQJXJOGLNCZEY-UHFFFAOYSA-N^Y
SMILES [He]
Properties
Chemical formula	He
Molar mass	4.002602 g·mol^−1
Appearance	Colourless gas
Boiling point	−269 °C (−452.20 °F; 4.15 K)
Thermochemistry
Std molar entropy (S^o298)	126.151-126.155 J K^−1 mol^−1
Pharmacology
ATC code	V03AN03 (WHO)
Hazards
S-phrases (outdated)	S9
Except where otherwise noted, data are given for materials in their standard state (at 25 °C [77 °F], 100 kPa).
N verify (what is ^YN ?)
Infobox references

Introduction

Schematic termscheme for Para- and Orthohelium with one electron in ground state 1s and one excited electron.

The quantum mechanical description of the helium atom is of special interest, because it is the simplest multi-electron system and can be used to understand the concept of quantum entanglement. The Hamiltonian of helium, considered as a three-body system of two electrons and a nucleus and after separating out the centre-of-mass motion, can be written as

${\displaystyle H({\vec {r}}_{1},\,{\vec {r}}_{2})=\sum _{i=1,2}{\Bigg (}-{\frac {\hbar ^{2}}{2\mu }}\nabla _{r_{i}}^{2}-{\frac {Ze^{2}}{4\pi \epsilon _{0}r_{i}}}{\Bigg )}-{\frac {\hbar ^{2}}{M}}\nabla _{r_{1}}\cdot \nabla _{r_{2}}+{\frac {e^{2}}{4\pi \epsilon _{0}r_{12}}}}$

where ${\displaystyle \mu ={\frac {mM}{m+M}}}$ is the reduced mass of an electron with respect to the nucleus, ${\displaystyle {\vec {r}}_{1}}$ and ${\displaystyle {\vec {r}}_{2}}$ are the electron-nucleus distance vectors and ${\displaystyle r_{12}=|{\vec {r_{1}}}-{\vec {r_{2}}}|}$. The nuclear charge, ${\displaystyle Z}$ is 2 for helium. In the approximation of an infinitely heavy nucleus, ${\displaystyle M=\infty }$ we have ${\displaystyle \mu =m}$ and the mass polarization term ${\textstyle {\frac {\hbar ^{2}}{M}}\nabla _{r_{1}}\cdot \nabla _{r_{2}}}$ disappears. In atomic units the Hamiltonian simplifies to

${\displaystyle H({\vec {r}}_{1},\,{\vec {r}}_{2})=-{\frac {1}{2}}\nabla _{r_{1}}^{2}-{\frac {1}{2}}\nabla _{r_{2}}^{2}-{\frac {Z}{r_{1}}}-{\frac {Z}{r_{2}}}+{\frac {1}{r_{12}}}.}$

It is important to note, that it operates not in normal space, but in a 6-dimensional configuration space ${\displaystyle ({\vec {r}}_{1},\,{\vec {r}}_{2})}$. In this approximation (Pauli approximation) the wave function is a second order spinor with 4 components ${\displaystyle \psi _{ij}({\vec {r}}_{1},\,{\vec {r}}_{2})}$, where the indices ${\displaystyle i,j=\,\uparrow ,\downarrow }$ describe the spin projection of both electrons (z-direction up or down) in some coordinate system.[2] It has to obey the usual normalization condition ${\displaystyle \sum _{ij}\int d{\vec {r}}_{1}d{\vec {r}}_{2}|\psi _{ij}|^{2}=1}$. This general spinor can be written as 2x2 matrix ${\displaystyle {\boldsymbol {\psi }}={\begin{pmatrix}\psi _{\uparrow \uparrow }&\psi _{\uparrow \downarrow }\\\psi _{\downarrow \uparrow }&\psi _{\downarrow \downarrow }\end{pmatrix}}}$ and consequently also as linear combination of any given basis of four orthogonal (in the vector-space of 2x2 matrices) constant matrices ${\displaystyle {\boldsymbol {\sigma }}_{k}^{i}}$ with scalar function coefficients

${\displaystyle \phi _{i}^{k}({\vec {r}}_{1},\,{\vec {r}}_{2})}$ as ${\displaystyle {\boldsymbol {\psi }}=\sum _{ik}\phi _{i}^{k}({\vec {r}}_{1},\,{\vec {r}}_{2}){\boldsymbol {\sigma }}_{k}^{i}}$. A convenient basis consists of one anti-symmetric matrix (with total spin ${\displaystyle S=0}$, corresponding to a singlet state)

${\displaystyle {\boldsymbol {\sigma }}_{0}^{0}={\frac {1}{\sqrt {2}}}{\begin{pmatrix}0&1\\-1&0\end{pmatrix}}={\frac {1}{\sqrt {2}}}(\uparrow \downarrow -\downarrow \uparrow )}$

and three symmetric matrices (with total spin ${\displaystyle S=1}$, corresponding to a triplet state)

${\displaystyle {\boldsymbol {\sigma }}_{0}^{1}={\frac {1}{\sqrt {2}}}{\begin{pmatrix}0&1\\1&0\end{pmatrix}}={\frac {1}{\sqrt {2}}}(\uparrow \downarrow +\downarrow \uparrow )\;;}$ ${\displaystyle {\boldsymbol {\sigma }}_{1}^{1}={\begin{pmatrix}1&0\\0&0\end{pmatrix}}=\;\uparrow \uparrow \;;}$ ${\displaystyle {\boldsymbol {\sigma }}_{-1}^{1}={\begin{pmatrix}0&0\\0&1\end{pmatrix}}=\;\downarrow \downarrow \;.}$

It is easy to show, that the singlet state is invariant under all rotations (a scalar entity), while the triplet can be mapped to an ordinary space vector ${\displaystyle (\sigma _{x},\sigma _{y},\sigma _{z})}$, with the three components

${\displaystyle \sigma _{x}={\frac {1}{\sqrt {2}}}{\begin{pmatrix}1&0\\0&-1\end{pmatrix}}}$, ${\displaystyle \sigma _{y}={\frac {i}{\sqrt {2}}}{\begin{pmatrix}1&0\\0&1\end{pmatrix}}}$ and ${\displaystyle \sigma _{z}={\frac {1}{\sqrt {2}}}{\begin{pmatrix}0&1\\1&0\end{pmatrix}}}$.

Since all spin interaction terms between the four components of ${\displaystyle {\boldsymbol {\psi }}}$ in the above (scalar) Hamiltonian are neglected (e.g. an external magnetic field, or relativistic effects, like angular momentum coupling), the four Schrödinger equations can be solved independently.[3]

The spin here only comes into play through the Pauli exclusion principle, which for fermions (like electrons) requires antisymmetry under simultaneous exchange of spin and coordinates

${\displaystyle {\boldsymbol {\psi }}_{ij}({\vec {r}}_{1},\,{\vec {r}}_{2})=-{\boldsymbol {\psi }}_{ji}({\vec {r}}_{2},\,{\vec {r}}_{1})}$.

Parahelium is then the singlet state ${\displaystyle {\boldsymbol {\psi }}=\phi _{0}({\vec {r}}_{1},\,{\vec {r}}_{2}){\boldsymbol {\sigma }}_{0}^{0}}$ with a symmetric function ${\displaystyle \phi _{0}({\vec {r}}_{1},\,{\vec {r}}_{2})=\phi _{0}({\vec {r}}_{2},\,{\vec {r}}_{1})}$ and orthohelium is the triplet state ${\displaystyle {\boldsymbol {\psi }}_{m}=\phi _{1}({\vec {r}}_{1},\,{\vec {r}}_{2}){\boldsymbol {\sigma }}_{m}^{1},\;m=-1,0,1}$ with an antisymmetric function ${\displaystyle \phi _{1}({\vec {r}}_{1},\,{\vec {r}}_{2})=-\phi _{1}({\vec {r}}_{2},\,{\vec {r}}_{1})}$. If the electron-electron interaction term is ignored, both spatial functions ${\displaystyle \phi _{x},\;x=0,1}$ can be written as linear combination of two arbitrary (orthogonal and normalized)

one-electron eigenfunctions ${\displaystyle \varphi _{a},\varphi _{b}}$:

${\displaystyle \phi _{x}={\frac {1}{\sqrt {2}}}(\varphi _{a}({\vec {r}}_{1})\varphi _{b}({\vec {r}}_{2})\pm \varphi _{a}({\vec {r}}_{2})\varphi _{b}({\vec {r}}_{1}))}$

or for the special cases

of ${\displaystyle \varphi _{a}=\varphi _{b}}$ (both electrons have identical quantum numbers, parahelium only): ${\displaystyle \phi _{0}=\varphi _{a}({\vec {r}}_{1})\varphi _{a}({\vec {r}}_{2})}$. The total energy (as eigenvalue of ${\displaystyle H}$) is then for all cases ${\displaystyle E=E_{a}+E_{b}}$ (independent of the symmetry).

This explains the absence of the ${\displaystyle 1^{3}S_{1}}$ state (with ${\displaystyle \varphi _{a}=\varphi _{b}=\varphi _{1s}}$) for orthohelium, where consequently ${\displaystyle 2^{3}S_{1}}$ (with ${\displaystyle \varphi _{a}=\varphi _{1s},\varphi _{b}=\varphi _{2s}}$) is the metastable ground state. (A state with the quantum numbers: principal quantum number ${\displaystyle n}$, total spin ${\displaystyle S}$, angular quantum number ${\displaystyle L}$ and total angular momentum ${\displaystyle J=|L-S|\dots L+S}$ is denoted by ${\displaystyle n^{2S+1}L_{J}}$.)

If the electron-electron interaction term ${\displaystyle {\frac {1}{r_{12}}}}$ is included, the Schrödinger equation is non separable. However, also if is neglected, all states described above (even with two identical quantum numbers, like ${\displaystyle 1^{1}S_{0}}$ with ${\displaystyle {\boldsymbol {\psi }}=\varphi _{1s}({\vec {r}}_{1})\varphi _{1s}({\vec {r}}_{2}){\boldsymbol {\sigma }}_{0}^{0}}$) cannot be written as a product of one-electron wave functions: ${\displaystyle \psi _{ik}({\vec {r}}_{1},\,{\vec {r}}_{2})\neq \chi _{i}({\vec {r}}_{1})\xi _{k}({\vec {r}}_{2})}$ — the wave function is entangled. One cannot say, particle 1 is in state 1 and the other in state 2, and measurements cannot be made on one particle without affecting the other.

Nevertheless, quite good theoretical descriptions of helium can be obtained within the Hartree–Fock and Thomas–Fermi approximations (see below).

Hartree–Fock method

The Hartree–Fock method is used for a variety of atomic systems. However it is just an approximation, and there are more accurate and efficient methods used today to solve atomic systems. The "many-body problem" for helium and other few electron systems can be solved quite accurately. For example, the ground state of helium is known to fifteen digits. In Hartree–Fock theory, the electrons are assumed to move in a potential created by the nucleus and the other electrons. The Hamiltonian for helium with two electrons can be written as a sum of the Hamiltonians for each electron:

${\displaystyle H=\sum _{i=1}^{2}h(i)=H_{0}+H^{\prime }}$

where the zero-order unperturbed Hamiltonian is

${\displaystyle H_{0}=-{\frac {1}{2}}\nabla _{r_{1}}^{2}-{\frac {1}{2}}\nabla _{r_{2}}^{2}-{\frac {Z}{r_{1}}}-{\frac {Z}{r_{2}}}}$

while the perturbation term:

${\displaystyle H'={\frac {1}{r_{12}}}}$

is the electron-electron interaction. H₀ is just the sum of the two hydrogenic Hamiltonians:

${\displaystyle H_{0}={\hat {h}}_{1}+{\hat {h}}_{2}}$

where

${\displaystyle {\hat {h}}_{i}=-{\frac {1}{2}}\nabla _{r_{i}}^{2}-{\frac {Z}{r_{i}}},i=1,2}$

E_ni, the energy eigenvalues and ${\displaystyle \psi _{n_{i},l_{i},m_{i}}({\vec {r}}_{i})}$, the corresponding eigenfunctions of the hydrogenic Hamiltonian will denote the normalized energy eigenvalues and the normalized eigenfunctions. So:

${\displaystyle {\hat {h}}_{i}\psi _{n_{i},l_{i},m_{i}}({\vec {r_{i}}})=E_{n_{i}}\psi _{n_{i},l_{i},m_{i}}({\vec {r_{i}}})}$

where

${\displaystyle E_{n_{i}}=-{\frac {1}{2}}{\frac {Z^{2}}{n_{i}^{2}}}{\text{ in a.u.}}}$

Neglecting the electron-electron repulsion term, the Schrödinger equation for the spatial part of the two-electron wave function will reduce to the 'zero-order' equation

${\displaystyle H_{0}\psi ^{(0)}({\vec {r}}_{1},{\vec {r}}_{2})=E^{(0)}\psi ^{(0)}({\vec {r}}_{1},{\vec {r}}_{2})}$

This equation is separable and the eigenfunctions can be written in the form of single products of hydrogenic wave functions:

${\displaystyle \psi ^{(0)}({\vec {r}}_{1},{\vec {r}}_{2})=\psi _{n_{1},l_{1},m_{1}}({\vec {r}}_{1})\psi _{n_{2},l_{2},m_{2}}({\vec {r}}_{2})}$

The corresponding energies are (in atomic units, hereafter a.u.):

${\displaystyle E_{n_{1},n_{2}}^{(0)}=E_{n_{1}}+E_{n_{2}}=-{\frac {Z^{2}}{2}}{\Bigg [}{\frac {1}{n_{1}^{2}}}+{\frac {1}{n_{2}^{2}}}{\Bigg ]}}$

Note that the wave function

${\displaystyle \psi ^{(0)}({\vec {r}}_{2},{\vec {r}}_{1})=\psi _{n_{2},l_{2},m_{2}}({\vec {r}}_{1})\psi _{n_{1},l_{1},m_{1}}({\vec {r}}_{2})}$

An exchange of electron labels corresponds to the same energy ${\displaystyle E_{n_{1},n_{2}}^{(0)}}$. This particular case of degeneracy with respect to exchange of electron labels is called exchange degeneracy. The exact spatial wave functions of two-electron atoms must either be symmetric or antisymmetric with respect to the interchange of the coordinates ${\displaystyle {\vec {r}}_{1}}$ and ${\displaystyle {\vec {r}}_{2}}$ of the two electrons. The proper wave function then must be composed of the symmetric (+) and antisymmetric(-) linear combinations:

${\displaystyle \psi _{\pm }^{(0)}({\vec {r}}_{1},{\vec {r}}_{2})={\frac {1}{\sqrt {2}}}[\psi _{n_{1},l_{1},m_{1}}({\vec {r}}_{1})\psi _{n_{2},l_{2},m_{2}}({\vec {r}}_{2})\pm \psi _{n_{2},l_{2},m_{2}}({\vec {r}}_{1})\psi _{n_{1},l_{1},m_{1}}({\vec {r}}_{2})]}$

This comes from Slater determinants.

The factor ${\displaystyle {\frac {1}{\sqrt {2}}}}$ normalizes ${\displaystyle \psi _{\pm }^{(0)}}$. In order to get this wave function into a single product of one-particle wave functions, we use the fact that this is in the ground state. So ${\displaystyle n_{1}=n_{2}=1,\,l_{1}=l_{2}=0,\,m_{1}=m_{2}=0}$. So the ${\displaystyle \psi _{-}^{(0)}}$ will vanish, in agreement with the original formulation of the Pauli exclusion principle, in which two electrons cannot be in the same state. Therefore, the wave function for helium can be written as

${\displaystyle \psi _{0}^{(0)}({\vec {r}}_{1},{\vec {r}}_{2})=\psi _{1}({\vec {r_{1}}})\psi _{1}({\vec {r_{2}}})={\frac {Z^{3}}{\pi }}e^{-Z(r_{1}+r_{2})}}$

Where ${\displaystyle \psi _{1}}$ and ${\displaystyle \psi _{2}}$ use the wave functions for the hydrogen Hamiltonian. [lower-alpha 1] For helium, Z = 2 from

${\displaystyle E_{0}^{(0)}=E_{n_{1}=1,\,n_{2}=1}^{(0)}=-Z^{2}{\text{ a.u.}}}$

where E${\displaystyle _{0}^{(0)}}$ = −4 a.u. which is approximately −108.8 eV, which corresponds to an ionization potential V${\displaystyle _{P}^{(0)}}$ = 2 a.u. (≅54.4 eV). The experimental values are E${\displaystyle _{0}}$ = −2.90 a.u. (≅ −79.0 eV) and V${\displaystyle _{p}}$ = 0.90 a.u. (≅ 24.6 eV).

The energy that we obtained is too low because the repulsion term between the electrons was ignored, whose effect is to raise the energy levels. As Z gets bigger, our approach should yield better results, since the electron-electron repulsion term will get smaller.

So far a very crude independent-particle approximation has been used, in which the electron-electron repulsion term is completely omitted. Splitting the Hamiltonian showed below will improve the results:

${\displaystyle H={\bar {H_{0}}}+{\bar {H'}}}$

where

${\displaystyle {\bar {H_{0}}}=-{\frac {1}{2}}\nabla _{r_{1}}^{2}+V(r_{1})-{\frac {1}{2}}\nabla _{r_{2}}^{2}+V(r_{2})}$

and

${\displaystyle {\bar {H'}}={\frac {1}{r_{12}}}-{\frac {Z}{r_{1}}}-V(r_{1})-{\frac {Z}{r_{2}}}-V(r_{2})}$

V(r) is a central potential which is chosen so that the effect of the perturbation ${\displaystyle {\bar {H'}}}$ is small. The net effect of each electron on the motion of the other one is to screen somewhat the charge of the nucleus, so a simple guess for V(r) is

${\displaystyle V(r)=-{\frac {Z-S}{r}}=-{\frac {Z_{e}}{r}}}$

where S is a screening constant and the quantity Z_e is the effective charge. The potential is a Coulomb interaction, so the corresponding individual electron energies are given (in a.u.) by

${\displaystyle E_{0}=-(Z-S)^{2}=-Z_{e}^{2}}$

and the corresponding wave function is given by

${\displaystyle \psi _{0}(r_{1}\,r_{2})={\frac {Z_{e}^{3}}{\pi }}e^{-Z_{e}(r_{1}+r_{2})}}$

If Z_e was 1.70, that would make the expression above for the ground state energy agree with the experimental value E₀ = −2.903 a.u. of the ground state energy of helium. Since Z = 2 in this case, the screening constant is S = 0.30. For the ground state of helium, for the average shielding approximation, the screening effect of each electron on the other one is equivalent to about ${\displaystyle {\frac {1}{3}}}$ of the electronic charge.[5]

Thomas–Fermi method

Not long after Schrödinger developed the wave equation, the Thomas–Fermi model was developed. Density functional theory is used to describe the particle density ${\displaystyle \rho ({\vec {r}}),\,r\,\epsilon \,\mathbb {R} ^{3}}$, and the ground state energy E(N), where N is the number of electrons in the atom. If there are a large number of electrons, the Schrödinger equation runs into problems, because it gets very difficult to solve, even in the atom's ground states. This is where density functional theory comes in. Thomas–Fermi theory gives very good intuition of what is happening in the ground states of atoms and molecules with N electrons.

The energy functional for an atom with N electrons is given by:

${\displaystyle \xi ={\frac {3}{5}}\gamma \int _{\mathbb {R} ^{3}}\rho ^{5/3}({\vec {r}})d^{3}{\vec {r}}\,+\int _{\mathbb {R} ^{3}}V({\vec {r}})\rho ({\vec {r}})d^{3}{\vec {r}}\,+{\frac {e^{2}}{2}}\int _{\mathbb {R} ^{3}}{\frac {\rho ({\vec {r}})\rho ({\vec {r'}})}{|{\vec {r}}-{\vec {r'}}|}}\,d^{3}{\vec {r}}d^{3}{\vec {r'}}}$

Where

${\displaystyle \gamma =(3\pi ^{2})^{2/3}{\frac {\hbar ^{2}}{2m}}}$

The electron density needs to be greater than or equal to 0, ${\displaystyle \int _{\mathbb {R} ^{3}}\rho =N}$, and ${\displaystyle \rho \rightarrow \xi }$ is convex.

In the energy functional, each term holds a certain meaning. The first term describes the minimum quantum-mechanical kinetic energy required to create the electron density ${\displaystyle \rho ({\vec {x}})}$ for an N number of electrons. The next term is the attractive interaction of the electrons with the nuclei through the Coulomb potential ${\displaystyle V({\vec {r}})}$. The final term is the electron-electron repulsion potential energy.[6]

So the Hamiltonian for a system of many electrons can be written:

${\displaystyle H=\sum _{i=1}^{N}{\Bigg [}-{\frac {\hbar ^{2}}{2m}}\nabla _{i}^{2}+V({\vec {r_{i}}}){\Bigg ]}+\int {\frac {e^{2}\rho ({\vec {r'}})}{|{\vec {r}}-{\vec {r'}}|}}d^{3}r'}$

For helium, N = 2, so the Hamiltonian is given by:

${\displaystyle H=-{\frac {\hbar ^{2}}{2m}}(\nabla _{1}^{2}+\nabla _{2}^{2})+V({\vec {r_{1}}},\,{\vec {r_{2}}})+\int {\frac {e^{2}\rho ({\vec {r'}})}{|{\vec {r}}-{\vec {r'}}|}}d^{3}r'}$

Where

${\displaystyle \int {\frac {e^{2}\rho ({\vec {r'}})}{|{\vec {r}}-{\vec {r'}}|}}d^{3}r'={\frac {e^{2}}{4\pi \epsilon _{0}}}{\frac {1}{|{\vec {r}}_{1}-{\vec {r}}_{2}|}},\,{\text{ and }}\,V({\vec {r_{1}}},\,{\vec {r_{2}}})={\frac {e^{2}}{4\pi \epsilon _{0}}}{\Bigg [}{\frac {2}{r_{1}}}+{\frac {2}{r_{2}}}{\Bigg ]}}$

yielding

${\displaystyle H=-{\frac {\hbar ^{2}}{2m}}(\nabla _{1}^{2}+\nabla _{2}^{2})+{\frac {e^{2}}{4\pi \epsilon _{0}}}{\Bigg [}{\frac {2}{r_{1}}}+{\frac {2}{r_{2}}}-{\frac {1}{|{\vec {r}}_{1}-{\vec {r}}_{2}|}}{\Bigg ]}}$

From the Hartree–Fock method, it is known that ignoring the electron-electron repulsion term, the energy is 8E₁ = −109 eV.

The variational method

To obtain a more accurate energy the variational principle can be applied to the electron-electron potential V_ee using the wave function

${\displaystyle \psi _{0}({\vec {r}}_{1},\,{\vec {r}}_{2})={\frac {8}{\pi a^{3}}}e^{-2(r_{1}+r_{2})/a}}$:

${\displaystyle \langle H\rangle =8E_{1}+\langle V_{ee}\rangle =8E_{1}+{\Bigg (}{\frac {e^{2}}{4\pi \epsilon _{0}}}{\Bigg )}{\Bigg (}{\frac {8}{\pi a^{3}}}{\Bigg )}^{2}\int {\frac {e^{-4(r_{1}+r_{2})/a}}{|{\vec {r}}_{1}-{\vec {r}}_{2}|}}\,d^{3}{\vec {r}}_{1}\,d^{3}{\vec {r}}_{2}}$

After integrating this, the result is:

${\displaystyle \langle H\rangle =8E_{1}+{\frac {5}{4a}}{\Bigg (}{\frac {e^{2}}{4\pi \epsilon _{0}}}{\Bigg )}=8E_{1}-{\frac {5}{2}}E_{1}=-109+34=-75{\text{ eV}}}$

This is closer to the experimental value, but if a better trial wave function is used, an even more accurate answer could be obtained. An ideal wave function would be one that doesn't ignore the influence of the other electron. In other words, each electron represents a cloud of negative charge which somewhat shields the nucleus so that the other electron actually sees an effective nuclear charge Z that is less than 2. A wave function of this type is given by:

${\displaystyle \psi ({\vec {r}}_{1},{\vec {r}}_{2})={\frac {Z^{3}}{\pi a^{3}}}e^{-Z(r_{1}+r_{2})/a}}$

Treating Z as a variational parameter to minimize H. The Hamiltonian using the wave function above is given by:

${\displaystyle \langle H\rangle =2Z^{2}E_{1}+2(Z-2){\Bigg (}{\frac {e^{2}}{4\pi \epsilon _{0}}}{\Bigg )}\left\langle {\frac {1}{r}}\right\rangle +\left\langle V_{ee}\right\rangle }$

After calculating the expectation value of ${\displaystyle {\frac {1}{r}}}$ and V_ee the expectation value of the Hamiltonian becomes:

${\displaystyle \langle H\rangle =\left[-2Z^{2}+{\frac {27}{4}}Z\right]E_{1}}$

The minimum value of Z needs to be calculated, so taking a derivative with respect to Z and setting the equation to 0 will give the minimum value of Z:

${\displaystyle {\frac {d}{dZ}}\left(\left[-2Z^{2}+{\frac {27}{4}}Z\right]E_{1}\right)=0}$

${\displaystyle Z={\frac {27}{16}}\sim 1.69}$

This shows that the other electron somewhat shields the nucleus reducing the effective charge from 2 to 1.69. So we obtain the most accurate result yet:

${\displaystyle {\frac {1}{2}}{\Bigg (}{\frac {3}{2}}{\Bigg )}^{6}E_{1}=-77.5{\text{ eV}}}$

Where again, E₁ represents the ionization energy of hydrogen.

By using more complicated/accurate wave functions, the ground state energy of helium has been calculated closer and closer to the experimental value −78.95 eV.[7] The variational approach has been refined to very high accuracy for a comprehensive regime of quantum states by G.W.F. Drake and co-workers[8][9][10] as well as J.D. Morgan III, Jonathan Baker and Robert Hill[11][12][13] using Hylleraas or Frankowski-Pekeris basis functions. One needs to include relativistic and quantum electrodynamic corrections to get full agreement with experiment to spectroscopic accuracy.[14][15]

Experimental value of ionization energy

Helium's first ionization energy is −24.587387936(25) eV.[16] This value was derived by experiment.[17] The theoretic value of Helium atom's second ionization energy is −54.41776311(2) eV.[16] The total ground state energy of the helium atom is −79.005151042(40) eV,[16] or −2.90338583(13) Atomic units a.u., which equals −5.80677166 (26) Ry.

See also

• Araki–Sucher correction
• Hydrogen molecular ion
• Lithium atom
• List of quantum-mechanical systems with analytical solutions
• Quantum field theory
• Quantum mechanics
• Quantum states
• Theoretical and experimental justification for the Schrödinger equation
• "Helium atom" on Wikiversity

References

1. For n = 1, l = 0 and m = 0, the wavefunction in a spherically symmetric potential for a hydrogen electron is ${\displaystyle \psi _{(}r)={\frac {1}{\sqrt {\pi }}}\left({\frac {Z}{a_{0}}}\right)^{\frac {3}{2}}\ e^{-{\textstyle {\frac {Zr}{a_{0}}}}}\;}$.[4] In atomic units, the Bohr radius ${\displaystyle {a_{0}}}$ equals 1, and the wavefunction becomes ${\displaystyle \psi _{(}r)={\frac {1}{\sqrt {\pi }}}Z^{\frac {3}{2}}\ e^{-{\textstyle Zr}}\;}$.

1. "Helium - PubChem Public Chemical Database". The PubChem Project. USA: National Center for Biotechnology Information.
2. P. Rennert, H. Schmiedel, C. Weißmantel. "Kleine Enzyklopädie Physik", VEB Bibliographisches Institut Leipzig, 1988, 192-194.
3. L.D. Landau, E.M. Lifschitz. "Lehrbuch der Theoretischen Physik", Bd. III (Quantenmechanik), Akademie-Verlag, Berlin 1971, Kap. IX, pp. 218
4. "Hydrogen Wavefunctions". Hyperphysics. Archived from the original on 1 February 2014.
5. B.H. Bransden and C.J. Joachain's Physics of Atoms and Molecules 2nd edition Pearson Education, Inc
6. http://www.physics.nyu.edu/LarrySpruch/Lieb.pdf
7. David I. Griffiths Introduction to Quantum Mechanics Second edition year 2005 Pearson Education, Inc
8. Drake, G.W.F.; Van, Zong-Chao (1994). "Variational eigenvalues for the S states of helium". Chemical Physics Letters. Elsevier BV. 229 (4–5): 486–490. doi:10.1016/0009-2614(94)01085-4. ISSN 0009-2614.
9. Yan, Zong-Chao; Drake, G. W. F. (1995-06-12). "High Precision Calculation of Fine Structure Splittings in Helium and He-Like Ions". Physical Review Letters. American Physical Society (APS). 74 (24): 4791–4794. doi:10.1103/physrevlett.74.4791. ISSN 0031-9007.
10. Drake, G. W. F. (1999). "High Precision Theory of Atomic Helium". Physica Scripta. IOP Publishing. T83 (1): 83–92. doi:10.1238/physica.topical.083a00083. ISSN 0031-8949.
11. J.D. Baker, R.N. Hill, and J.D. Morgan III (1989), "High Precision Calculation of Helium Atom Energy Levels", in AIP ConferenceProceedings 189, Relativistic, Quantum Electrodynamic, and Weak Interaction Effects in Atoms (AIP, New York),123
12. Baker, Jonathan D.; Freund, David E.; Hill, Robert Nyden; Morgan, John D. (1990-02-01). "Radius of convergence and analytic behavior of the 1/Z expansion". Physical Review A. American Physical Society (APS). 41 (3): 1247–1273. doi:10.1103/physreva.41.1247. ISSN 1050-2947.
13. Scott, T. C.; Lüchow, A.; Bressanini, D.; Morgan, J. D. III (2007). "The Nodal Surfaces of Helium Atom Eigenfunctions" (PDF). Phys. Rev. A. 75 (6): 060101. Bibcode:2007PhRvA..75f0101S. doi:10.1103/PhysRevA.75.060101. hdl:11383/1679348.
14. Drake, G. W. F.; Yan, Zong-Chao (1992-09-01). "Energies and relativistic corrections for the Rydberg states of helium: Variational results and asymptotic analysis". Physical Review A. American Physical Society (APS). 46 (5): 2378–2409. doi:10.1103/physreva.46.2378. ISSN 1050-2947.
15. G.W.F. Drake (2006). "Springer Handbook of Atomic, molecular, and Optical Physics", Edited by G.W.F. Drake (Springer, New York), 199-219.
16. Kramida, A., Ralchenko, Yu., Reader, J., and NIST ASD Team. "NIST Atomic Spectra Database Ionization Energies Data". Gaithersburg, MD: NIST.CS1 maint: uses authors parameter (link)
17. D. Z. Kandula, C. Gohle, T. J. Pinkert, W. Ubachs, and K. S. E. Eikema (2010). "Extreme Ultraviolet Frequency Comb Metrology". Phys. Rev. Lett. 105 (6): 063001. arXiv:1004.5110. Bibcode:2010PhRvL.105f3001K. doi:10.1103/PhysRevLett.105.063001. PMID 20867977.CS1 maint: uses authors parameter (link)