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The Emission Directionality of Electronic Intraband Transitions in Stacked QuantumDots
Alexander Mittelstadt,∗ Ludwig A. Th. Greif, and Andrei SchliwaInstitut fur Festkorperphysik, Technische Universitat Berlin,
Hardenbergstr. 36, 10623 Berlin, Germany(Dated: August 20, 2021)
We investigate the emission directionality of electronic intraband (intersubband) transitions instacked coupled quantum dots. Using a well-established eight-band k · p method, we demonstratethat the minor contributions from the valence band mixing into the conduction band govern thepolarization and emission directionality of electronic p-to-s-type intraband transitions. Despite thatthe contribution from the central-cell part to the momentum matrix element is dominant, we find,the contribution from the matrix elements among the envelope functions cannot be neglected. Withthe help of an artificial cuboidal quantum dot, we show that the vertical emission from intrabandtransitions can be tuned via the emitter’s vertical aspect ratio. Subsequently, we show that theseresults can be transferred to more realistic geometries of quantum dots and quantum dot stacksand demonstrate that the vertical emission can be enhanced from 23 % to 46 % by increasing theemitter’s vertical aspect ratio to the isotropic case with a vertical aspect ratio of 1.0. Therefore, astacking of a few quantum dotss (∼4 for the investigated structures) is already sufficient to improvethe vertical radiation significantly. Additionally, we discuss the impact of the number of stackedQDs as well as the effect of the interdot coupling strength on the radiation properties.
Compact semiconductor light emitters and detectorsoperating within the infrared spectrum gained interestwithin last years as terahertz devices provide the highfrequencies needed, e.g., for next generation wireless com-munications systems; see Refs. [1–5]. Widely tunable in-traband (intersubband) transitions in quantum dot (QD)heterostructures can play a crucial role in the develop-ment of suitable infrared devices, whereas QD semicon-ductor devices also show high temperature stability andnarrow linewidths; cf. [6–9]. In addition, since infraredintraband transitions in quantum well devices are for-bidden for light polarized perpendicular to the growthdirection (normal incident light), QD-based systems arebetter suited for infrared sensors (IR photo detectors)[10–15], low-threshold terahertz vertical-cavity surface-emitting lasers [16, 17], and photovoltaic [18–21].In contrast to the polarization of interband transitions insingle and stacked QDs (see, e.g., Refs. [22–31]), a com-prehensive study of the polarization and emission proper-ties of intraband transitions of QD stacks is still missing.Studies on single QDs and stacks of two QDs (forminga QD molecule) show that electronic intraband transi-tions in QDs exhibit a fundamentally different spatialemission as interband transitions [32–37]. As well, Sheng found that the polarization of intraband transitionscan be explained by the symmetry of valence band func-tions, in other words, by directed interactions of the lo-cal atomic orbitals. It was also found that the mixing ofthese valence band functions into the conduction bandstates is different for a QD molecule compared to a sin-gle QD, giving rise to other transition matrix elements
. Based on these preliminary findings on transitionmatrix elements, we show a comprehensive study of theradiation properties of stacked QDs, guiding the designand growth of such QD structures, potentially makinginfrared devices more efficient. Although polarization-resolved transition matrix elements can be derived anal-ogous to interband transitions [30, 31, 38–42], which inturn can be used to calculate angle-resolved radiationintensities , studies investigating the emission direc-tionality of intraband transitions of QD stacks are stilllacking. In this article, we focus on the vertical aspectratio (AR) of the emitter as we found that the emitter’sconfinement region’s aspect ratio has a decisive impact onthe emission direction of the intraband transitions sim-ilar to that of the interband transitions. By stackingQDs, ensembles of 30 and more vertically coupled QDscan be formed, changing the emitter’s AR and where theinterdot coupling strength is adjusted via the separatingbarrier width [24, 43, 44].This article is organized as follows: First, we outline themethod of calculating the QDs electronic structure andthe determination of the radiation pattern of CB intra-band transitions. Next, we examine three different se-ries of QDs and highlight the effect of changing the QDstack’s morphology on its radiation pattern. Series Aconsists of artificial cubodial QDs, which help to iden-tify the impact of the QDs AR on emission propertiesof stacked QDs; see Fig. 1(a). Series B and C are usedto compare our findings with series A with more realisticQD structures: Here, stacks of InGaAs/GaAs QDs are in-vestigated, mapping the most basic parameters changingthe AR of the spatial confinement and the QDs couplingstrength, showing that the findings from Series A can betransferred to realistic structures. In Series B, we demon-strate the impact of the number of QDs stacked. Here,for closely stacked QDs, the stack number is varied from
radial distance in hQDIn
Figure 1. (a) The QD structures investigated. Series A:nine artificial cubodial QDs with AR between 1.6 and 0.4.Series B: stacks of ten identical QDs to a single QD withbarrier width of b = 0 monolayers (MLs). Series C: stacksof nine identical QDs with barriers varying from b = 0 MLsto b = 16 MLs. (b) Scheme of the modeled QD geometrywith a gradual composition. The Indium x content withinan InxGa1−xAs QD as a function of the distance to the apexcenter in units of the QD’s height hQD.
a single QD to a stack of ten QDs. For series C, for astack of five QDs, the interdot distance and thus the QDcoupling strength is changed from closely stacked intoa weak coupling regime until the QDs decouple. For se-ries B and C, InxGa1−xAs QDs are modeled as truncatedpyramids with a side-wall inclination of 40, embedded ina GaAs matrix, in agreement with investigations in Refs.[45, 46]. The model QDs have a base diameter of 17.5 nmand a height of 3.4 nm, in agreement with experimentalinvestigations of stacked InAs QDs [28, 43, 47, 48]. Theindium content decreases linearly (see Fig. 1(b)) in agree-ment with experimental investigations and findings thatuniform compositions are not able to reproduce the cor-rect electron-hole alignment and polarization propertiesfor interband transitions [49–54].
II. METHOD OF CALCULATION
Calculations of the emission directionality of intrabandCB transitions in stacks of up to ten QDs are build onan established 8-band k · p model; see Refs. [33, 55, 56].By using the k ·p model, electronic structure calculationsof extended QD systems are more efficient compared toatomistic models. Furthermore, long-range interactionslike strain and strain-induced piezoelectricity are consid-ered, which usually have to be omitted by atomistic the-ories; cf. Refs. [57–60] and references therein. In theeffective mass approximation, single-particle states arerepresented as a product basis
|φk〉 |uk〉 , (1)
with the envelope |φk〉 and the atomic-like bandedge (Γ-point) Bloch functions
|u〉 = [|s ↑〉 , |x ↑〉 , |y ↑〉 , |z ↑〉 , |s ↓〉 , |x ↓〉 , |y ↓〉 , |z ↓〉]T ,(2)
where the arrows denote the spin and the |s〉, |x〉 , |y〉 , |z〉denote the s- and p-type bandedge Bloch functions, re-spectively. It is also possible to transform the Bloch ba-sis into another set of eigenfunctions of the Hamiltonian,which represent the states in a conduction (CB) and va-lence band (VB) Bloch basis; see Refs. [61–63]. For ex-ample, considering quantization along the z-axis,
i |s ↓〉|x〉+i|y〉√
|x〉−i|y〉√3|↑〉 − |z〉√
where the dots represent the functions |cb2〉, |hh2〉, |lh2〉,and |so2〉 build from bandedge Bloch functions with op-posite spin in Eq. 2 and |cb1〉 = |ucb ↓〉, and so on. Here,the |cb〉 denote the CB and the |hh〉, |lh〉, and |so〉 theheavy, light, and splitoff VB states, respectively. In gen-eral, any state |ψ〉 can be represented in this basis set byprojection onto the respective basis functions
| 〈uk|ψ〉 |2 = | |φk〉 |2 . (4)
The lattice mismatch of InAs and GaAs (about 7%) re-sults in a highly strained heterostructure shifting the CBvia the deformation potentials ac, av, and b; cf. Refs.[63, 64]. The simplified equation in Ref.  illustratesthe strain-induced band coupling for the CB
VCB = ECB + aceh (5)
and the VB VVB = EVB + aveh ± b2eb, where ECB and
EVB are the unstrained CB edges, respectively. The ehand eb are the hydrostatic and biaxial strain components,respectively. Thus, the hydrostatic strain is shifting theCB’s energetic position, while in contrast, the VB is alsoinfluenced by the biaxial strain resulting in a splitting ofthe light- and heavy-hole band. Consequently, the con-finement region and the strain determine the characterof the hole ground state, i.e., the leading |hh〉 and |lh〉contributions, respectively, which have a decisive influ-ence on the polarization of the electron-hole decay .In contrast to the hole ground state, the lowest CB stateis less affected by the strain (see Ref. ) and the enve-lope’s symmetry is not changed. The leading contribu-tions of the CB states is, at least for the InGaAs/GaAsQD systems considered, always s-like, but the VB statesmix into the states and influence the polarization of theCB intraband transitions and thus their radiation char-acteristics; cf. Refs. [34, 35, 63]. Similar to the change
of the VB groundtate’s composition considered for inter-band transitions (see Ref. ), the |hh〉 and |lh〉 contri-bution of the CB groundstate change for stacks of QDswith different heights and spacings. This is particularlyrelevant as enlarged |hh〉 or |lh〉 contributions result inenhanced horizontal or vertical plus horizontal polariza-tion of the intraband transitions, respectively, owing tothe different components from the bandedge Bloch func-tions; cf. Eq. 3.In Fermi’s golden rule, the matrix element for a transi-tion between state |i〉 and state |j〉 using the expansionin Eq. 1 is
〈j|ε · p|i〉 =∑kl=1
δkl 〈φjk|ε · p|φil〉︸ ︷︷ ︸(a)
〈φjk|φil〉 〈ujk|ε · p|uil〉︸ ︷︷ ︸(b)
where |j〉 = |ψj〉. While interband transitions aregoverned by the second term (b) and are calculatedvia the optical matrix elements of the bandedge Blochfunctions, considering intraband transitions non of bothterms might be neglected, whereby the matrix element(a) is calculated from the envelope functions involved,i.e., 〈ujk|uil〉 = 1. The emission rate is
Γi,j(ε) ∝∣∣∣[(a) + (b)]
∣∣∣2 . (7)
We derive the rate of emitted photons Γi,j as a func-tion of their polarization ε(φε, θε) and their propagationdirection k(φk, θk) by assuming a transversal propaga-tion. Using a frame of reference ρ, ϕ, ϑ (in spherical co-ordinates), with the z′-axis aligned to the propagationdirection k, the integrated transition rate for all possi-ble polarizations can be written as a line integral in theϑ = π/2-plane
[ ∫ 2π
dϕΓi,j(ϕ, π/2)]. (8)
Here, o is the sum over all degenerate intraband states |ψ〉considered for the transition. Throughout this article, weuse a spatially resolved emission intensity parametrizedin the QD’s frame of reference using the condition ε ·k =0. Equation 8 simplifies to
where φk and θk define the propagation direction. If therate Γi,j(k) is calculated, each transition is counted sev-eral times, thus, the rate is normalized to the total rateof emitted photons. We calculate the degree of radiationanisotropy (DORA) for the three perpendicular crystalplanes. Here, we use, analogously to the degree of po-larization defined in Refs. [23, 24, 30, 41], the (110)- and
vertical aspect ratio
no strainx,y z(b)
Figure 2. (a) Decomposition of the lowest conduction bandstate of the cubodial QD series A into the |cb〉 (blue circles),|hh〉 (green empty square), |lh〉 (green filled square), and |so〉(red pyramid) basis functions versus vertical aspect ratio. (b)Corresponding decomposition into the atomic-like basis func-tions |x〉, |y〉 (blue pyramid), and |z〉 (red inverted pyramid).Both diagrams are calculated excluding effects of strain.
(110)-plane as an indicator for the degree of the QD sys-tems top- and in-plane-emission:
DORA(001) =Γ(k = )− Γ(k = )
Γ(k = ) + Γ(k = )(10)
DORA(110) =Γ(k = )− Γ(k = )
Γ(k = ) + Γ(k = )(11)
DORA(110) =Γ(k = )− Γ(k = )
Γ(k = ) + Γ(k = )(12)
III. DISCUSSION AND RESULTS
As discussed above, interband transitions are governedby the central-cell term Eq. 6(b). If we now assumethat intraband transitions to be governed by Eq. 6(a),the trivial conclusion would be that CB px,y-to-s-type,| |ψs〉 |2 and | |ψpx,y
〉 |2, respectively, transitions absorb oremit light polarized within the (001)-plane. However,previous numerical investigations using eight-band k · pmodels and calculating intraband dipole matrix elementsreveal that for QDs, the term Eq. 6(b) is much larger(about an order of magnitude) than the term (a) calcu-lated from the envelopes involved; cf. Refs. [32, 34]. As aconsequence, the envelope part is neglected by previousinvestigations of single QDs and QD molecules (see Refs.[34, 35]), where an approximation for the dipole moment,which contains the central-cell term solely, is used; see,e.g., Ref. . In agreement with previous investigations,we find for the QD series investigated that the transitiondipole moment calculated via term Eq. 6(b) is larger (byabout a factor of three to four) than the dipole momentcalculated from (a); see Fig. 4. As such our calculationsdemonstrate that term (a) has a not negligible impact onthe polarization of the CB intraband transitions; there-fore, the whole dipole moment is considered within oursimulations of the radiation anisotropy via Eq. 9.
Figure 3. Diagrams are calculated including effects of strain and strain-induced internal fields. (a) Decomposition of the lowestconduction band (CB) state of the cubodial QD series A into the |cb〉 (blue circles), |hh〉 (green empty square), |lh〉 (greenfilled square), and |so〉 (red pyramid) basis functions versus vertical aspect ratio (AR). (b) A plot of the energies for the threecorresponding Kramers-degenerate electron states, i.e., the px,y- (semi-filled circles) and s-type orbitals (filled circles), wheres-type state refers to | |ψs〉 |2, likewise for the excited states. The right y-axis shows the hydrostatic strain expectation valuefor the lowest CB state (orange diamonds), i.e., εh = 〈ψ1|εh|ψ1〉. (c and d) Plots of the conduction band edge VCB (black) andthe hydrostatic strain εh (orange) for the cubodial QDs with AR = 1.6 (c) and with AR = 0.4 (d).
A. The role of aspect ratio.
With the help of the series of artificial cubic QDs, weshow that the geometry of the confinement region alonechanges the radiation pattern. Therefore, we calculatedseries A without and with strain. Figure 2(a) shows thedifferent contributions of the VB functions |hh〉, |lh〉, and|so〉 to the lowest CB state without strain. Changing theQDs AR results in altering contributions of |hh〉 and |lh〉for AR > 1 and AR < 1 , while the |so〉 contributionremains more or less constant. In contrast to interbandtransitions, the atomic-like basis functions |x〉, |y〉, and|z〉 in Fig. 2(b) do not reflect the prevalent confinementregion, but as expected, the |x, y〉 and |z〉 fractions aredegenerate at AR = 1. The contribution of the |z〉 ba-sis function decreases with growing AR, while the |x, y〉contribution slightly decreases. In this regard, intrabandtransitions show a different characteristic compared tointerband transitions.Including strain and strain induced fields, the findings arevery similar; see Fig. 3(a). Here, also an enhancement ofthe |hh〉 and a reduction of the |lh〉 contribution withincreasing AR is observed. As discussed in Sec. II, theincreasing |hh〉-contribution results in an enhanced in-plane polarization, whereas, on the other hand, a larger|lh〉-contribution also raises the polarization within thegrowth direction z. Within the region of confinement, theCB edge shifts to higher energies the larger the hydro-static strain, and again, the hydrostatic strain becomesstronger the larger the region of confinement; see Figs.3(c,d) as well as Refs. [22, 65] for QD stacks. As a result,the contribution of the VB functions to the lowest CBstate is reduced and, likewise, its leading contribution,|cb〉-like, is increased. Similarly, an increasing AR re-duces the conduction-band-valence-band mixing; see Fig.3(a). The shift of the CB edge and the hydrostatic strainas a function of aspect ratio is also reflected in the evolu-tion of the energy eigenvalues of the first three Kramers-
vertical aspect ratio
(110) (a) (b)
Figure 4. (a) Relative share of the term (a) (blue pyra-mid) and term (b) (red inverted pyramid) contributing to thetransition dipole moment in Eq. 7 for the cubodial QD se-ries A versus aspect ratio. (b) DORA(110) of the term (a)(blue pyramid) and (b) (red inverted pyramid) in Eq. 7, re-spectively. The green axis depicts the contribution of the|hh〉 (green empty square) and |lh〉 (green filled square) basisfunctions from Fig. 3(a).
degenerate CB states; see Fig. 3(b). The p-to-s transitionenergies shift blue with increasing AR, raising the tran-sition matrix element Eq. 6. The hydrostatic strain ex-pectation value for the lowest CB state εh = 〈ψ1|εh|ψ1〉is increasing with AR reflecting the decreasing energyeigenvalues of the CB states.Figure 4(a) shows the relative shares of the transitiondipole moments in Eq. 7(a) versus (b) in the total dipolemoment for the py-to-s transitions of QDs in series A. Asthe AR increases, term (b) gains slightly over (a), with2.9 times greater than (a) for an AR = 1.6. Figure 4(b)shows the in-plane radiation DORA(110) determined viaEq. 11 for the terms (a) and (b), respectively. Also, thechange in the |hh〉 and |lh〉 components of the lowest CBstate from Fig. 3(a) is shown to illustrate the change interm (b) from nearly isotropic radiation for AR < 1.0to a radiation pattern perpendicular to (001)-plane forAR > 1.0. Term (a), in contrast, remains constant ata value of DORA(110) = −0.34, caused, as expected,by a strong anisotropic in-plane dipole moment of the
Figure 5. (a–e, k–o) normalized radiated power (Prad) persolid angle of the first and last QD structures within seriesA, B, and C, respectively. Blue and red radiation patternscorrespond to DORA(110) and DORA(110), respectively. (f–j) DORA(110) (blue semi-filled circle) and DORA(110) (redsemi-filled circle) of all QD structures investigated. As thesymmetry axis of the p-type are perpendicular to each other,the blue and red semi-filled circles correspond also to py- andpx-type CB states, respectively.
p-to-s transitions. This changes only minimally for anAR = 1.0, which is caused by the distinct shape of theinvolved orbitals for the artificial cubic QD at symmet-ric spatial confinement. Term (b) alone thus reflects thechange in the QD confinement region, resulting in en-hanced radiation perpendicular to the growth plane forQDs with AR > 1.0.The combined impact of terms (a) and (b) on the emis-sion directionality of series A is depicted in Figs. 5(a,f,k),
which results in a slightly more pronounced DORA ofDORA(110) & −46% for a AR > 1.0 compared to the in-dividual contributions of terms (a) and (b) shown in Fig.4(b). Figure 5(a) shows the radiation pattern within the(110)-plane at an AR = 1.6, which is highly anisotropicresulting from a strong in-plane polarization for the py-to-s transition. Compared to interband transitions (seeRef.  for AR < 1.0), intraband transitions at anAR > 1.0 result in a slightly more pronounced top emis-sion, which makes the contribution of the term (a) in Eq.7 apparent. For aspect ratios AR < 1.0, DORA is in-creasing, reflecting the growing |lh〉 contribution to thelowest CB state, but still making top emission more ef-fective than in-plane due to the term Eq. 7(a); see Fig.5(k). In Figure 6 (series A), the absolute values of thebasis functions |cb〉, |hh〉, |lh〉, and |so〉 orbitals are shownfor the vertical aspect ratios AR = 1.6, AR = 1.0, andAR = 0.4 in the (001)-plane. Here, |cb〉 is the sum of |cb1〉and |cb2〉, likewise for the other three basis functions. Forall ARs, the |hh〉-contribution exhibits a 4-fold symmetrywith a central node, resulting in a significant overlap withthe CB p-type orbitals. The |lh〉-contribution changes itssymmetry slightly from s-like for ARs < 1.0 to a mixtureof a 4-fold and s-like symmetry for ARs ≥ 1.0 withouta central node. Despite the |so〉-contribution is barelyinfluenced by changing the AR (cf. Figs. 2(a) and 3(a)),its symmetry changes from an s-like to a 4-fold symme-try with a central node for aspect rations AR < 1.0 and≥ 1.0, respectively. Due to the change in symmetry of the|so〉 basis function, the overlap with the p-type orbitalsincreases with aspect ratio, albeit not as pronounced asfor the |hh〉 function.
B. The role of number of stacked QDs.
In the second series we investigate the emission direc-tionality versus the number of stacked dots. We choosea barrier width of b = 0 for this series, as it representsthe maximal interdot coupling. Similarly, by omittingthe barrier, the influence of the AR on the emission pat-tern can be analyzed, also allowing a direct comparisonwith series A. Furthermore, experimental findings sug-gest that columnar QDs may stay in contact with eachother, if they were grown with a barrier of a few MLs[24–26].Figures 5(g,h) show the DORA values within the (110)-and (110)-plane for the py-to-s and px-to-s transitions,respectively. Beginning with a stack of four QDs, theemission directionality changes with further stackingfrom nearly isotropic for the single QD with DORA ≈−2% to a strong top emission with DORA > −36%.The change from an isotropic to a strongly anisotropicemission direction thus reflects the changing contribu-tions of the VB functions, with the |lh〉 contributionchanging to a predominant |hh〉 contribution for a stackof four QDs. We define a collective vertical aspectratio via the number of stacked QDs, ARcol(nQD) =
series: |cb〉 |hh〉 |lh〉 |so〉
A: AR = 1.6
C: b = 0ML
B: # = 10
A: AR = 1.0
A: AR = 0.4
B: # = 4
B: # = 1
C: b = 8ML
C: b = 16ML
Figure 6. The absolute values of the lowest conduction bandstate basis envelopes |cb〉, |hh〉, |lh〉, and |so〉 for three selectedgeometries of series A, B, and C in the (001)-plane integratedalong the -axis and normalized to the maximum in eachsubfigure. Structures not shown resemble the symmetries ofthe envelopes depicted, e.g., AR = 1.6 resembles the symme-tries for aspect ratios larger than 1.0 and AR = 0.4 for ARssmaller than 1.0.
nQDhQD/(average QD width), which allows us to com-pare the ARcol with the AR from series A. As for series A,the emission directionality can be tuned to a strong topemission by stacking QDs to ARcol(nQD) ≥ 1.0; for ourseries B, the aspect ratio for four QDs is ARcol(4) = 0.92.Figures 5(b,c) and (l,m) depict the corresponding emis-sion patterns for a stack of ten QDs and a single QD,respectively, showing a strong top emission for stackswith nQD ≥ 4. Figures 5(g,h) also depict the DORAvalues for radiation parallel to the axis of the py and px-type orbitals, respectively, showing an isotropic radiationpattern, becoming slightly anisotropic for stacks of QDs
smaller than four. The symmetries of the VB functionsfor series B in Fig. 6 follow the same pattern as for seriesA.
C. The role of interdot separation.
With help of the last series C, we investigate the im-pact of increasing the interdot barrier b on the emissiondirectionality of stacked QDs. If QDs are stacked closelywith b = 0 MLs, a strong top emission with DORA val-ues of ≈ −40% are observed for a stack of five QDs; cf.Fig. 5(i,j). Figures 5(d,e) and (n,o) depict the radiationpattern for b = 0 MLs and b = 16 MLs, respectively.By increasing the interdot separation, the |hh〉- and |lh〉contributions shift towards the single QD case of SeriesB, or AR = 0.4 for series A. As shown in Ref. , theband structure and strain distribution is almost identi-cal to an uncoupled single QD. In contrast to series B,the emission directionality changes linearly from a strongtop to a more isotropic emission of DORA ≈ −15% and≈ 4%, respectively; cf. Fig. 5(i,j). The envelopes in Fig.6 show identical symmetries as for series B, despite the|so〉-contribution at b = 8 MLs showing a state changingfrom an s-like to a 4-fold symmetry. We note, however,that an anti-binding s-type state forms as the QDs sep-aration is increased, which would make measuring theradiation characteristics of the p-s transitions even moredifficult for stacks with large barriers; cf. Refs. .
We demonstrate that the vertical emission of intra-band transitions of stacked QDs can be tuned via thestructure’s vertical aspect ratio. With the help of anartificial cuboidal QD, we show that the minor contri-butions from the central-cell part within the momentummatrix element change with aspect ratio enhancing orweakening the emission anisotropy. In contrast to inter-band transitions, the strain has a subordinate role andthe change of the aspect ratio itself results in a moredominant |lh〉/|hh〉 contribution of the lowest CB state.In addition, we find that the matrix elements amongthe envelope functions have a significant contribution tothe emission direction of stacked QDs and cannot be ne-glected.We investigate two series of QDs, investigating the im-pact of (i) the number of stacked QDs on the radiationpattern and (ii) the coupling strength between stackedQDs. Here we show that the results for the artificialQD can be transferred to realistic QD structures. In QDstacks, stacking QDs leads to a larger aspect ratio, thusenhancing the top emission for the CB intraband transi-tion, although this is only beneficial up to the isotropicwith an AR of 1.0, as further stacking then provides noadditional enhancement. Moreover, we show that thevertical emission is enhanced with increasing AR, vice
versa to the interband transitions in QDs. By increasingthe interdot distance in QD stacks, i.e., weakening theQD coupling strength, the emission pattern converges toa single QD, reducing the vertical emission to a moreisotropic pattern.Similar to interband transitions, our calculations showqualitative changes in the radiation pattern of QD stacksand provide qualitative values of the degree of radiationanisotropy (DORA) for the parameters considered. Inaddition, we provide insight into the contribution of theenvelope functions versus the central cell fraction to theemission rate and pattern. Our calculations also considerthe contribution of the envelope functions to the emission
pattern, which has been neglected in previous studiesof the polarization of intraband transitions as its con-tribution is comparatively small. Therefore, our studiesprovide new insight into the radiation anisotropy of QDintraband transitions, especially for stacked QDs, whichmay be beneficial for designing future infrared deviceswith enhanced in-plane or top emission polarization.
The authors would like to thank Dirk Ziemann forreading the manuscript and for the fruitful and construc-tive discussions.
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